text:
\section*{Abstract}
\else \normalsize
\fi}

\def\if@twocolumn\fi\par\clearpage{\if@twocolumn\fi\par\clearpage}

\tabcolsep 12pt
 \makeatother
\noncompletefalse\typeout{** FINAL form}
\refphysrevtrue
\renewcommand{\baselinestretch}{1.4}

\begin{document}
\title{Effects of Instantons on the Excited Baryons \\
and Two-Nucleon Systems}
\author{Sachiko Takeuchi}
\affiliation{
Department of Public Health and Environmental Science,\\
School of Medicine,
Tokyo Medical and Dental University,\\
1-5-45  Yushima, Bunkyo, Tokyo 113, Japan}
\date{\today}
\maketitle
{\bf Abstract:~~}
The effects of the spin-orbit and the tensor parts of
the instanton-induced interaction
on the excited nonstrange baryons up to $N$=2
and on the two-nucleon systems are investigated.
The spin-orbit force from the instanton-induced interaction
cancels most of that from the one-gluon exchange
in the excited baryons
while the spin-orbit force in the nucleon systems remains strong
after the inclusion of the instanton-induced interaction.
The model including the spin-orbit and the tensor terms
of the instanton-induced interaction
as well as the one-gluon exchange is found to reproduce successfully
the excited baryon
mass spectrum and the scattering phase shifts of two nucleons
in the spin-triplet
relative $P$-wave state.

\noindent
PACS numbers:
14.20.Gk, 13.75.Cs, 12.38.Lg, 12.39.Jh.

\newpage

\section{Introduction}

Valence quark models
have been applied to low-energy light-quark systems and found to be
successful in
reproducing major properties of the hadrons and hadronic systems.
The reason why
such models can be so successful
is not well understood.
The empirical approach, however, suggests a few reasons.
One of them is that the model space has an appropriate symmetry.
Another reason is that a light quark has rather heavy
effective mass.
In such a low energy region,
the effects of
complicated configurations such as $q\bar q$ excitation and
 dynamical gluon effects are
considered to be taken into account by employing
constituent valence quarks and effective interactions among quarks
with the required symmetry.

These empirical models usually
contains three terms:
the kinetic term, the confinement term, and the
effective one-gluon exchange (OGE) term.
It is considered that OGE stands for the
perturbative gluon effects and that the confinement force represents
the long-range nonperturbative gluon effects.

It is well known
that the color magnetic interaction (CMI) in OGE
is responsible to produce many of the hadron properties.
By adjusting the strength of OGE,
CMI can reproduce
the hyperfine splittings (HFS,
e.g., ground state N-$\Delta$ mass difference)
 \cite{GS76,IK78,Is92,SS90}
as well as the short range repulsion of
the two-nucleon systems in the relative $S$-wave
\cite{MYO84,TSY89,Sh89}.
It, however, is also known that
the strength of OGE determined in this
empirical way is much greater than 1, which makes it hard
to treat it as the perturbative effect.

Moreover, the valence quark model including only OGE
as an origin of HFS
has a spin-orbit problem.
The spin-orbit part of OGE is strong; it is just strong enough
to explain the observed large spin-orbit force between two nucleons
\cite{MYO84,TSY89}.
On the other hand,
the experimental mass spectrum of the excited baryons,
N$^*$ and $\Delta^*$
resonances, indicates
that such a strong spin-orbit force should not exist between quarks.
A valence quark model in which the spin-orbit parts
of the quark-quark
 interaction are removed by hands
can well simulate the  observed mass spectrum
\cite{GS76,IK78,Is92,SS90}.
It was pointed out that the confinement force also
produces the spin-orbit force, which may cancel the one from OGE
in the excited baryons \cite{IK78}.
Suppose one takes the spin-orbit part of a
 two-body confinement force into account, however,
it also cancels the spin-orbit part of OGE
in the nuclear force \cite{MYO84}.
To explain both of the features at the same time
is highly nontrivial.

The instantons were originally introduced in  relation to
the $U_A$(1) problem;
their coupling to the surrounding light-quark zero modes
produces the flavor-singlet interaction between quarks,
which leads the observed large mass difference
of $\eta'$-$\eta$ mesons \cite{tH76,Sh84}.
How this instanton-induced interaction (\mbox{\rm I\thinspace I\thinspace I}),
which contributes by a few hundred MeV in the
meson sector, affects in other hadron systems
is an interesting problem.
Actually, several recent works
indicate  that the effect is also large
in the baryon sector\cite{Ko85,OT91,TO91,Ta94,MT91,Negele}.
It is hard to determine the strength of the instanton effects
quantitatively directly from QCD.
The above empirical works on \mbox{\rm I\thinspace I\thinspace I}\ can contribute  also in
understanding the structure of the QCD vacuum.
We argue that a valence quark model should include \mbox{\rm I\thinspace I\thinspace I}\ as a
short-range nonperturbative gluon effect
in addition to the other aforementioned gluon effects.

In ref.\ \cite{Ta94}, we demonstrated that
introducing \mbox{\rm I\thinspace I\thinspace I}\ may solve the above
difficulty in the $P$-wave systems due to  the cancellation between
OGE and \mbox{\rm I\thinspace I\thinspace I}.
In this paper, we discuss
effects of the noncentral parts, especially the spin-orbit part of
\mbox{\rm I\thinspace I\thinspace I}\ on the excited nonstrange baryons up to $N=2$
and on the two-nucleon systems.
 We employ a quark potential model  for that purpose
because it can deal both with the single baryons and
with the two-nucleon systems, and because the discussion
based on the symmetry can be performed more clearly
for the present subject.
In section 2, we will show the model hamiltonian.
The discussion based on the symmetry is presented in section 3.
The numerical results are shown in section 4.
The discussion and the summary are in section 5.
The complicated wave functions and the matrix elements
are summarized in the appendix.

\section{Quark Model with Instanton Induced Interaction}

We assume that both of OGE and \mbox{\rm I\thinspace I\thinspace I}\
are included in the quark model hamiltonian:
\begin{eqnarray}
H_{\rm quark}
&=&
 K+(1-p_{\rm III})V_{\rm OGE} + p_{\rm III} \mathbox(V_{\rm III})\ + V_{\rm conf}\, ,
\label{eq:quarkmodel}
\end{eqnarray}
where $p_{\rm III}$ is a parameter which represents the rate of
the $S$-wave N-$\Delta$
mass difference explained by \mbox{\rm I\thinspace I\thinspace I}.
 When one introduces the
interaction strong enough to give the observed $\eta$-$\eta'$ mass
difference, $p_{\rm III}$ becomes 0.3--0.4
\cite{OT91,TO91,Ta94}.
$V_{\rm OGE}$ and
\mathbox(V_{\rm III})\
are the Galilei invariant terms of the \mbox{\rm I\thinspace I\thinspace I}\ and OGE potentials.

According to
the instanton liquid model, the size of instantons is about 0.3 fm,
which is a new scale of the low energy QCD phenomena \cite{Sh84}.
The instantons and the anti-instantons couple
to flavor-singlet light quarks.
Assuming the instanton is small enough
comparing to the system we consider,
one obtains the effective interaction between quarks
arising from that coupling
 as \cite{tH76,Ko85,OT91,TO91,Ta94}:
\begin{equation}
 \mathbox(H_{\rm III}) = V_0^{(2)}  \sum_{i<j}
   \bar\psi_R(i) \bar\psi_R(j) \,
             {15 \over 8} {\cal A}^{flavor}_{ij}
                ( 1- {1 \over 5} \mbfsig_i\cdot\mbfsig_j )
                          \,\psi_L(j) \psi_L(i)
                          + \hbox{(h.c.)} , \hfill
\label{relaIII}
\end{equation}
where $V_0^{(2)}$ is the strength of the two-body part of \mbox{\rm I\thinspace I\thinspace I}.
We obtain the following potential
performing the nonrelativistic reduction
to the lowest non-vanishing order in $(p/m)$
for each operator of different spin structure \cite{Ta94}:
\begin{eqnarray}
\mathbox(V_{\rm III}) &=&
 V_0^{(2)}  \sum_{i<j}{\cal A}^{flavor}_{ij}
         \left[{15\over16}\!\left(1\!-\!{1\over 5} \mbfsig_i\cdot\mbfsig_j \right)
-{1 \over m^{2}} \!\left( {3\over4}
LS
+{q^2\over12}(1\!-\!{3\over16}\lambda_i\cdot\lambda_j)S_{12}\right)
\right]
\\
&=& V_0^{(2)}  \sum_{i<j}
       \!\left(1+{3\over32}\lambda_i\cdot\lambda_j+\!{9\over 32}
       \lambda_i\cdot\lambda_j\mbfsig_i\cdot\mbfsig_j \right)
\nonumber\\
&&-{\cal A}^{flavor}_{ij}
{1 \over m^{2}} \!\left( {3\over4}
LS
+{q^2\over12}(1\!-\!{3\over16}\lambda_i\cdot\lambda_j)S_{12}\right)
 .
\label{eq:Hiii}
\end{eqnarray}
The same procedure for OGE leads \cite{MYO84,DGG75}
\begin{equation}
V_{\rm OGE} = 4\pi\alpha_s \sum_{i<j}{(\lambda_i\cdot\lambda_j)\over 4}\!
         \left[{1\over q^2}-{\mbfsig_i\cdot\mbfsig_j\over6m^{2}}
+{3\over 2m^2q^{2}}LS
+{1\over12m^2}S_{12}
\right]
\label{eq:Hoge}\\
\end{equation}
with
\begin{eqnarray}
LS&=&
{(\mbf(\sigma)_i+\mbf(\sigma)_j)}\cdot i[\mbf(q)\times{(\mbf(p)_i-\mbf(p)_j)}]/4
\\
S_{ij}& =&
3(\mbf(\sigma)_i\cdot \mbf(q))(\mbf(\sigma)_j\cdot \mbf(q))/q^2-(\mbfsig_i\cdot\mbfsig_j) .
\end{eqnarray}
Here ${\cal A}^{flavor}_{ij} =(1-P^{flavor}_{ij})/2$
is the antisymmetrizer in the flavor space,
$m_{u}=m_{d}\equiv m$ is a constituent quark mass,
and $\mbf(q)$ is the three momentum transfer.
The values of
 $m$, the strength of each interaction, $\alpha_s$
and $V_0^{(2)}$,
with the size parameter $b$ of the quark core of the baryon,
are listed in table 1.
These values are chosen as follows \cite{MYO84,TSY89,OT91,TO91,Ta94}:
the quark mass is $\FRAC{1}{3}$ of the nucleon mass;
the size parameter
$b$ is taken to be a little smaller
than the real nucleon size reflecting that
the observed baryon size has contribution from the meson cloud;
$\alpha_s$ and $V_0^{(2)}$
are determined to give the ground state
N-$\Delta$ mass difference $\mu$
\begin{equation}
{4\over 3\sqrt{2\pi}}{\alpha_s\over m_u^2b^3}
= -{9\over 4 \sqrt{2\pi}^3}{V_0^{(2)} \over b^3}
= 293 {\rm MeV} \equiv \mu~~;
\label{eq6}
\end{equation}
$a_{\rm conf}$, the strength of the confinement potential,
can be determined by
$\delta m_{N}/\delta b = 0$;
and $p_{\rm III}$ is taken to give the $\eta'$-$\eta$ mass difference.

\section{Symmetry}

One of the reasons that the nonrelativistic quark model
can successfully
predict the properties of the low energy system is
that the model has an appropriate symmetry.
We discuss here whether the observed properties in
the spin-orbit force, small  in the single baryons
and large in the two-nucleon systems, can be
explained by discussion based on the symmetry.

The interactions (\ref{eq:Hiii}) and (\ref{eq:Hoge}) consist of
 operators which conserve the flavor symmetry.
Thus,
the spin-orbit or the tensor part
of the two-body interactions for a quark pair,
which requires the quark pair to be symmetric in the spin space,
can be decomposed as follows:
\begin{eqnarray}
{\cal O} &=& {\overline {\cal O}}^A + {\cal O}^S + {\overline {\cal O}}^S + {\cal O}^A,
\label{eq:projop}
\end{eqnarray}
where
\begin{eqnarray}
{\overline {\cal O}}^A  & \equiv &
{\cal O}{\cal A}^{orb} {\cal S}^{spin} {\cal A}^{color} {\cal A}^{flavor} \\
{\cal O}^S  & \equiv &
{\cal O} {\cal A}^{orb} {\cal S}^{spin} {\cal S}^{color} {\cal S}^{flavor}
\\
{\overline {\cal O}}^S  & \equiv &
{\cal O} {\cal S}^{orb} {\cal S}^{spin} {\cal A}^{color} {\cal S}^{flavor}
\\
{\cal O}^A  & \equiv &
{\cal O}{\cal S}^{orb} {\cal S}^{spin} {\cal S}^{color} {\cal A}^{flavor}
\end{eqnarray}
with antisymmetrizers ${\cal A}$'s and symmetrizers ${\cal S}$'s.
For a quark pair with the relative-odd partial wave,
the first two terms in the right hand side of
eq.\ (\ref{eq:projop}) are relevant, while the last two terms are
for relative-even partial-wave pairs.
The operator with bar is for color singlet pairs,
which is relevant to the single baryons.
Those for the flavor-singlet (-octet) quark pairs
are marked by $A$ ($S$).

The noncentral term of \mbox{\rm I\thinspace I\thinspace I}\ contains
only flavor-singlet components,
 ${\overline {\cal O}}^A$ and ${\cal O}^A$;
OGE has all of the component in eq.\ (\ref{eq:projop}).
Since OGE is vector-particle exchange and \mbox{\rm I\thinspace I\thinspace I}\
is alike to scalar-particle exchange,
their noncentral term has an opposite sign.
Thus, there is a spin-orbit cancellation where both of OGE
and \mbox{\rm I\thinspace I\thinspace I}\ survives.
Namely, it occurs only for the flavor-singlet quark pairs:
the odd-partial wave pairs in color-singlet systems
and the even-partial wave pairs in color-octet systems.

To see the properties of the single baryons
and of the short range part of the
two-nucleon systems,
we evaluate the energy of systems by the gaussian wave functions
where the center-of-mass motion is eliminated:
$(0p)(0s)^2$ for the negative-parity single baryons,
$(1s)(0s)^2$, $(0p)^{2}(0s)$ and
$(0d)(0s)^2$ for the positive-parity single baryons, and
 and $(0p)(0s)^5$
for the six-quark systems.

In Table 2, the contribution of matrix element
of each operator is listed (see appendix)
for the negative-parity baryon N$^{*}$($\FRAC{5}{2}^{-}$),
for the positive-parity excited baryon N$^{*}$($\FRAC{7}{2}^{+}$),
and for the six-quark state
with the relative $P$-wave two-nucleon quantum number.
Once the parameters are taken to satisfy eq.(\ref{eq6}), the
contribution can be expressed in units of $\mu$ together with the
dimensionless parameter $mb$.
The contribution of the color symmetric operator, i.e.,
the operator without a bar,
is found to be dominant in the six-quark state.
Since there is no cancellation for that operator,
the spin-orbit reduction of the relative $P$-wave two-nucleon systems
 is small.
Within the single baryon, of course,
only the operators with a bar are relevant.
The OGE-\mbox{\rm I\thinspace I\thinspace I}\
cancellation occurs in the spin-orbit part operating
on the odd-wave quark pairs
in the single baryons.
It is the
spin-orbit force between
the odd-wave quark pairs
that should disappear in the single baryon
as we will show in the next section.
Thus, we expect that this cancellation will
lead the observed properties in
the spin-orbit force.

\section{Results and Discussions}
\subsection{Single Baryons}

We investigate the mass spectrum of the excited nonstrange baryons
by a nonrelativistic quark model with the spin-spin, the spin-orbit
and the tensor parts of OGE
and \mbox{\rm I\thinspace I\thinspace I}.
The central spin-independent part has been modified.
The central part of the original model hamiltonian
eq.\ (\ref{eq:NRHamiltonian})
does not produce the correct zeroth-order splitting
seen in the positive parity $N$=2 baryons.
It is mainly because the spin-independent contact interaction
from the one-gluon
exchange is strong and has a wrong sign.
As ref.\ \cite{GS76,IK78,Is92} pointed out,
the deviation of the spin-independent force
from harmonic will be much important and be expressed by the
following parameterization.
We use the same method in ref.\ \cite{Is92}
with the same values except for a little modified $E_{0}$:
\begin{eqnarray}
H_{quark} &=& H_c + (1-p_{\rm III}) \widetilde{\mathbox({V_{\rm OGE}})}
+p_{\rm III} \widetilde{\mathbox(V_{\rm III})}
\label{eq:NRHamiltonian}\\
H_c &=& E_0 + N \Omega + \delta \;U
\\
E_0 &=& 1090 ~{\rm MeV}~+p_{\rm III} \; \mu/2
\\
\Omega &=& 440~{\rm MeV}
\\
\delta  &=& 400~{\rm MeV}
\\
U&=& \left\{\matrix{-1 \cr -{1\over2} \cr -{2\over5} \cr
-{1\over5} \cr 0 }\right.
 ~~{\rm for}~~({\rm D}^{SF},L^P)=
 \left\{\matrix{(56',0^+) \cr (70,0^+) \cr (56,2^+)
 \cr (70,2^+) \cr {\rm otherwize} }\right.
{}~~,
\end{eqnarray}
where $\widetilde{\mathbox({V_{\rm OGE}})}$ ($\widetilde{\mathbox(V_{\rm III})}$) is
the spin-spin, the spin-orbit and
the tensor part of $\mathbox({V_{\rm OGE}})$ ($\mathbox(V_{\rm III})$).

Our results in this subsection are affected by only few
parameters: $E_0$ to give the ground state energy,
$\Omega$ to give the difference among
the ground states, the $N$=1 negative-parity baryons
and the $N$=2 positive-parity baryons,
$\delta$ to split the $N$=2 baryons, $\mu$ in
 eq.(\ref{eq6}) for the hyperfine splittings,
$(m_{u}b)^2$, and $p_{\rm III}$ to give the relative strength of \mbox{\rm I\thinspace I\thinspace I}.
This
estimate by the harmonic oscillator wave function is affected
only by the above combinations of the parameters listed in table 1.
The values of the parameters here are
reasonable.  $E_0$ is close to $3m_u$,
and the strength of OGE $\alpha_s(1-p_{\rm III})$
becomes smaller when $p_{\rm III}$ = 0.4.

In Fig.\ 1a) and b), the mass spectra of
the negative-parity and the positive parity baryons are shown.
The ground state mass is kept 940 MeV
for the nucleon and 1240 MeV for $\Delta$ in each parameter set.
The observed mass spectrum
is shown by stars (the weighted average of the observed values)
and boxes (possible error) \cite{Data}.
The number of the stars corresponds to
reliability of existence of the states:
the four-star state means that
its existence is certain while the one-star state
means that evidence of its existence is poor.

The next right to the experiment
is the mass spectrum given by $H_c$.
This three-parameter model gives an excellent prediction for the
excited baryons.
The third spectrum is derived from the hamiltonian which contains
$H_c$ and the tensor term of OGE ($p_{\rm III}=0$):
it corresponds to the one in ref.\ \cite{IK78,Is92},
where the spin-orbit term is omitted by hand.
The introduction of the tensor term
gives little change in the spectrum.
Actually, one cannot conclude that the tensor term
is necessary only from the
mass spectrum; it was included so as
to give correct decay modes \cite{KI80}.

The fourth column contains the central,
the spin-spin and the spin-orbit term with $p_{\rm III} =0$.
The spectrum, especially for the nucleons,
is destroyed completely;
 which is the reason why the spin-orbit term
 had to be removed in ref.\ \cite{IK78,Is92}.
The question is, however, whether all the spin-orbit terms
should be removed or not.
The excited $\Delta^{*}$ mass spectrum
is better than the nucleons'.  There, all the quark pairs
are  in the flavor symmetric; the spin-orbit term exists only
for the relative $0d$-wave pairs.

The hamiltonian of the fifth spectrum
is the same as the fourth one except that
we remove all the spin-orbit force between
the relative $0p$-wave quark pairs,
namely, flavor-singlet pairs.
The remaining spin-orbit term affects only
the relative $0d$-quark pairs.
The excited nucleon spectrum changes drastically;
most of the spin-orbit effects,
which destroy the spectrum,
are found to come from the relative $0p$-wave quark pairs.
The remaining effects of the spin-orbit force are
still somewhat stronger than the best fit, but
the spectrum becomes much more closer to the realistic one.

As we showed in the previous section, the spin-orbit force between
the relative odd partial wave pairs reduces by introducing \mbox{\rm I\thinspace I\thinspace I}.
The sixth column corresponds to the hamiltonian
(\ref{eq:NRHamiltonian}) with
$p_{\rm III}$ = 0.4;
it includes the central (parameterized),
the spin-spin, the spin-orbit
and the tensor terms of both OGE and \mbox{\rm I\thinspace I\thinspace I}.
In this choice, the strength of the spin-orbit force between
$0p$-pairs reduces by 0.32 from the $p_{\rm III} =0$ case
while that between $0d$-pairs reduces by $(1-p_{\rm III})=0.6$.
Note that this simple model does
only have six parameters ($E_0$, $D_0$, $\delta$, $\mu$, $(m_ub)^2$
and $p_{\rm III}$) for the whole nonstrange baryons up to the
$N$=2 including both of the positive parity
and the negative parity states.
We do not adjust the relative strength of
the spin-spin, the spin-orbit and the tensor term.
The result is reasonably consistent with the
experiments.
Thus, we can conclude that the flavor-singlet interaction
plays an essential role
in reducing the strong spin-orbit force in
the excited baryons to the observed strength.

In ref.\ \cite{IK78,Is92,KI80},
the tensor part of OGE was introduced
so as to give an appropriate decay rates.
One of their examples is the relative strength of the
$\pi$N decay from two $\Delta$($\FRAC{5}{2}^+$):
$\Delta$(1905) and $\Delta$(2000).
We estimate the ratio of the decay matrix elements for those states
using the transition operator defined in \cite{KI80},
where they assumed the pointlike pion is emitted from single quark.
The calculated matrix element for the
higher $\Delta$($\FRAC{5}{2}^+$)
is found by about 30\% smaller
than that of the lower state.
The experimental partial decay width
of the lower energy state to the
$\pi$N channel is 32 to 39 MeV;
two experiments are reported
for the decay width from the higher energy state:
 5 and 28 MeV \cite{Data}.
It seems that the higher state
decays more weakly to $\pi$N than the lower state.
This decay-rate ratio for these states is
consistent with the experiments,
though it should be considered as a very rough estimate.

A possible flaw of our model as well as that in
ref.\ \cite{IK78,Is92,KI80} is $\Delta$($\FRAC{3}{2}^+$).
Two $\Delta$($\FRAC{3}{2}^+$) are seen experimentally:
$\Delta$(1600) and $\Delta$(1920);
both of them decay to the $\pi$N
channel rather strongly.
The lowest energy level of the predicted states is 1734 MeV.
Inclusion of the spin-orbit term and \mbox{\rm I\thinspace I\thinspace I}\ has made the state
lower by about 150 MeV,
but the level is still higher than it should be by about 100 MeV.
The estimated decay matrix elements from
both of the two lower states
to the  $\pi$N channel are large, but that from the highest level
is small.
The couplings to the baryon-meson channel,
such as N$\pi$, may be important
 \cite{Fu93}.
The experiments have a large error also for these states.
Further investigation  both in the
experiments and in the theories is necessary to clarify this problem.

\subsection{Two Nucleons}

The main purpose of this paper is to show the inclusion of the
instanton induced interaction
gives the channel specific cancellation of
the spin-orbit force between quarks.
In the symmetry consideration we show that
the spin-orbit force in the two-nucleon scattering
does not reduce much by introducing \mbox{\rm I\thinspace I\thinspace I}.
In this section we show that a realistic
quark cluster model including
\mbox{\rm I\thinspace I\thinspace I}\
can actually reproduce the two-nucleon scattering phase shift
for the triplet $P$-wave states.

The wave function is the same as those in ref.\
\cite{MYO84,TSY89,TO91}:
\begin{equation}
	\Psi = {\cal A}_{q}\{\phi^{2}_{N}\chi(R)\} ~~.
\end{equation}
The notation is the same as that in the appendix,
except for $\chi(R)$, the relative wave function,
which is now to be solved.

The hamiltonian for the valence quarks
is eq.(\ref{eq:quarkmodel}), except that
we omit the tensor terms of OGE and \mbox{\rm I\thinspace I\thinspace I}\
because the tensor force
between the quarks is not dominant
in the two-nucleon system \cite{TSY89}.
We use the linear confinement potential for $V_{\rm conf}$
in eq.(\ref{eq:quarkmodel}):
\begin{equation}
	V_{\rm conf} = \sum_{i<j} \: a_{\rm conf}\; r_{ij} ~~.
\end{equation}
After integrating out the internal coordinates of the nucleons,
 we have the resonating group method equation:
\begin{eqnarray}
	\{ H_{q}+N^{1/2}V_{\rm EMEP}N^{1/2}-EN\}\chi  & = & 0
	\label{eq:RGMeq}
\end{eqnarray}
with $H_{q}$ is the hamiltonian kernel for $H_{quark}$,
 N is the normalization kernel.
The effective meson exchange potential, $V_{\rm EMEP}$,
is multiplied by $N^{1/2}$
because the potential $V_{\rm EMEP}$ should be added
to the equation in the Schr\"odinger form.
Here we take $V_{\rm EMEP}$ to have the central
and the tensor parts of
the one-pion exchange with
the form factor corresponding to the size parameter $b$,
and the gaussian-type central attraction \cite{TSY89}:
\begin{eqnarray}
	V_{\rm EMEP}(R) & = &
	(\tau\cdot\tau)(\sigma\cdot\sigma) V_{\pi}^{C}(R)+
	(\tau\cdot\tau) V_{\pi}^{T}(R)\;S_{12}+V_{g}(R)
	\label{eq:EMEP}
	\\
	V_{\pi}^{C}(R) & = &
	 {g^{2}_{\pi}\over 4\pi}{1\over 3}
	 \left({m_{\pi}\over2m_{N}}\right)^{2}
{\exp[-m_{\pi}R]\over R}
{1\over 2}\{ {\rm Erfc}(\alpha_{-})
- \exp[2m_{\pi}R]{\rm Erfc}(\alpha_{+})  \}
\\
	V_{\pi}^{T}(R) & = & {g^{2}_{\pi}\over 4\pi}
	{1\over 3} \left({m_{\pi}\over2m_{N}}\right)^{2}
{\exp[-m_{\pi}R]\over R} {1\over 2}
	\left[\left\{1+{3\over m_{\pi}R}+
	{3\over (m_{\pi}R)^{2}}\right\}
	   {\rm Erfc}(\alpha_{-}) \right.
\nonumber\\
&-& \left\{1-{3\over m_{\pi}R}
+{3\over (m_{\pi}R)^{2}}\right\}\exp[2m_{\pi}R]{\rm Erfc}(\alpha_{+})
\nonumber\\
&-&\left.\left\{1+{6\beta\over(m_{\pi}R)^{2}}\right\}
{m_{\pi}R\over \sqrt{\pi\beta^{3}}} \exp[-\alpha_{-}^{2}] \right]
	\\
\alpha_{\pm} & = & {m_{\pi} b \over \sqrt{3}}
\pm {\sqrt{3} R \over 2b}
\\
\beta &=& (m_{\pi} b)^{3}/3
\\
	V_{g}(R)&=&
	V_{\sigma}
	\exp\left[-\left({R\over r_{\sigma}+r_{a}}\right)^{2}\right]
	-\{V_{\sigma}+V_{\pi}^{C}(0)\}
	\exp\left[-\left({R\over r_{\sigma}-r_{a}}\right)^{2}\right] ~~.
\end{eqnarray}
The parameters $V_{\sigma}$ and $r_{\sigma}$ in $V_{\rm EMEP}$
are determined
by fitting the experimental phase shifts of
the triplet partial-odd wave states
with  fixed $r_{a}$  (table 1.)
 The coupling constant
$g^{2}_{\pi}/(4\pi)=13.7$ is taken from ref.\ \cite{SAID}.
The other parameters
in $H_{quark}$ are the same as in the previous section,
which are also listed in table 1.

To see the contribution from the spin-orbit term more clearly,
we recompile the phase shift as \cite{MYO84,TSY89}
\begin{eqnarray}
	\delta(^{3}P_{C}) & = &
	{1\over9}\delta(^{3}P_{0})+{1\over3}\delta(^{3}P_{1})
	+{5\over9}\delta(^{3}P_{2})
\\
	\delta(^{3}P_{T}) & = &
-{5\over36}\delta(^{3}P_{0})+{5\over24}\delta(^{3}P_{1})
-{5\over72}\delta(^{3}P_{2})
\\
	\delta(^{3}P_{LS}) & = &
-{1\over6}\delta(^{3}P_{0})-{1\over4}\delta(^{3}P_{1})
+{5\over12}\delta(^{3}P_{2}) ~~.
\end{eqnarray}

The calculated phase shifts are shown in fig.\ 3
together with those of the
energy-dependent phase shift analysis for the low-energy region,
VZ40, taken from SAID database \cite{SAID}.
The central part seems to require more sophisticated
effective meson exchange than the two-ranged gaussian
potential.
The one-pion exchange can give enough strength to
the tensor part of the two-nucleon system.
The spin-orbit force is reproduced by
the quark model well, even when \mbox{\rm I\thinspace I\thinspace I}\ is included by $p_{\rm III} = 0.4$.
As seen in table 2, the cancellation occurs only
for the color-singlet
quark pairs, which play minor role
in the $P$-wave two-nucleon systems.
The \mbox{\rm I\thinspace I\thinspace I}\ spin-orbit part for the color-singlet pairs
has the same sign as that of OGE.
Thus, the reduction of the spin-orbit effect
by including \mbox{\rm I\thinspace I\thinspace I}\ is less than
$(1-p_{\rm III})$.

\section{Discussion and Summary}

We investigate the effects of the noncentral part
of the instanton induced interaction
on the excited nonstrange baryons and two nucleon systems.
It is found that \mbox{\rm I\thinspace I\thinspace I}\ spin-orbit force cancels
the OGE spin-orbit force in the excited baryons
while the spin-orbit force in the two nucleon systems
remains strong after the
inclusion of \mbox{\rm I\thinspace I\thinspace I}.

The other possible source of the noncentral part
is the confinement force.
Such a channel specific cancellation, however,
occurs because that \mbox{\rm I\thinspace I\thinspace I}\ only affects
the flavor-singlet quark pairs.
The two-body confinement force, which has
the factor $(\lambda\cdot\lambda)$,
shows similar channel dependence to OGE and cannot produce
the cancellation required here.

The meson-exchange also produces the noncentral parts.
Usually, the $\sigma$,
$\rho$ and $\omega$ mesons are considered
as the main source of the spin-orbit force between
the nucleons.
This picture, however, cannot be applied
to the quark systems in a straightforward way.
These mesons are not pointlike; one cannot safely assume
that they
interact directly to quarks.
Moreover, their couplings to the nucleons are determined
mainly from the two-nucleon scattering data empirically.
In a model which includes only meson and baryon degrees of freedom,
the $\omega$N coupling is usually taken to be strong so
as to produce the short-range
repulsion between two nucleons.
In a quark model the repulsion is explained
 by the quark Pauli-blocking effect, by OGE and by \mbox{\rm I\thinspace I\thinspace I}.
The $\sigma$-meson exchange, which produces
the intermediate attraction,
also stands for complicated modes such as two-pion exchange,
coupling to the
$\pi\Delta$ channel, and even the attraction from \mbox{\rm I\thinspace I\thinspace I}.
It is hard to determine the genuine coupling to the mesons.
Here we take a quark-meson hybrid picture;
the short-ranged properties are explained
by the nature of a quark model
and the long-ranged properties are explained
by the meson-exchange model.
The modes which can be presented by the mesons
are taken into account as
the meson clouds.
The $\rho$-meson cloud has similar dependence
to OGE because
$(\tau\cdot\tau)$ shows similar channel dependence
to $(\lambda\cdot\lambda)$;
it will not produce the channel-specific cancellation to OGE.
The spin-orbit force of the $\omega$ or $\sigma$ cloud
 may produce such a cancellation.
Their strength, however, becomes smaller in such a picture.
 The contribution from meson clouds is unlikely
 to produce large effects required here.

On the contrary, there is a clear evidence for
the existence of the interaction
between the flavor-singlet quarks in the meson mass spectrum,
i.e.\ $\eta'$-$\eta$
mass difference;
this effect is considered to come not from the meson exchange
but from  the instanton-light quark coupling,
whose role we investigate here.
It is natural to think that there are large effects from \mbox{\rm I\thinspace I\thinspace I}\
also on the
 properties of the baryons or baryon systems, one of which,
 we argue,
 is the cancellation in the spin-orbit and the tensor force.

 The spin-orbit and the
 tensor part of \mbox{\rm I\thinspace I\thinspace I}\ survives only
 for the color-singlet quark pairs
 in a relative-odd partial wave state or
 for the color-octet quark pairs in a relative-even
 partial wave state.
 There, the cancellation of the spin-orbit and tensor parts
 occurs between OGE and \mbox{\rm I\thinspace I\thinspace I};
 which leads the particular cancellation required.
The relative strength of each term may change if we take
into the higher order relativistic effects account.
 The channel-specific cancellation is, however,
 explained based on the symmetry;
the overall nature will still be valid
with the change of the model parameters.

 This discussion based on the symmetry have to
 be reexamined when one considers
 the relativistic systems or the systems including strangeness.
 The estimate by  the MIT bag model indicates that
the major effect of the cancellation still exists
in the negative-parity baryons
\cite{Ta94}.
It is interesting to investigate the role of
the instanton induced interaction
in the excited baryons with the strangeness,
especially in the flavor-singlet states,
which will be presented in elsewhere.
\bigskip

This work was supported in part by Grant-in-Aid
for Encouragement of Young Scientists (A) (No.\ 07740206),
for General Scientific Research (No.\ 04804012)
and for Scientific Research on Priority Areas (No.\ 05243102)
from the Ministry of Education, Science, Sports and Culture.

\newpage
\section*{
Appendix A: Matrix Elements by the harmonic oscillator wave
functions}
Here we evaluate each operator defined by eq.\ (\ref{eq:projop}).

\subsection{Single Baryons}
\subsubsection{Wave functions}

\noindent{\it a) $S$-wave baryons}

There are flavor-decuplet states with $J^P=\FRAC{3}{2}^+$
and flavor-octet
states with $\FRAC{1}{2}^+$.
 By writing the orbital angular momentum, $L$, and
intrinsic spin, S, explicitly with the dimension
in the flavor space, {\bf D}$^{F}$,
and the dimension in the spin-flavor space,  D$^{SF}$,
as $|{\bf D}^{F};D^{SF}(LS)J^{P}\rangle$, they are represented as:
\begin{eqnarray}
|1\rangle \equiv \left|{\bf 10};56\left(0\half(3)\right)\half(3)^{+}
\right\rangle
& = & |[1^3]^C\rangle  |[3]^O \rangle  |[3]^F \rangle |[3]^S \rangle
\label{eq:31}
\\
|2\rangle \equiv \left|{\bf 8};56\left(0\half(1)\right)\half(1)^{+}
\right\rangle
& = & |[1^3]^C\rangle  |[3]^O \rangle
 \{|[21]^F \rangle  |[21]^S \rangle\}_{[3]} ~~.
\end{eqnarray}

\noindent{\it b) $P$-wave baryons}

There are flavor-decuplet states with $J^P=\FRAC{1}{2}^-$,
$\FRAC{3}{2}^-$ and flavor-octet
states with $J^P=(\FRAC{1}{2}^-)^{2}$, $(\FRAC{3}{2}^-)^{2}$,
$\FRAC{5}{2}^-$.  For a
future use,  we listed flavor-singlet states with
$\FRAC{1}{2}^-$, $\FRAC{3}{2}^-$
for the strangeness $-1$ systems.  In the same representation above,
they are:
\begin{eqnarray}
|3\rangle \equiv \left|{\bf 10};70\left(1\half(1)\right)J^{-}
\right\rangle
& = &
|[1^3]^C\rangle \{ |[21]^O \rangle |[3]^F \rangle |[21]^S \rangle \}_{[3]}
\\
|4\rangle \equiv \left|{\bf 8};70\left(1\half(3)\right)J^{-}
\right\rangle
& = &
|[1^3]^C\rangle \{ |[21]^O \rangle |[21]^F \rangle  \}_{[3]} |[3]^S \rangle
\\
|5\rangle \equiv \left|{\bf 8};70\left(1\half(1)\right)J^{-}
\right\rangle
& = &
|[1^3]^C\rangle \{ |[21]^O \rangle |[21]^F \rangle |[21]^S \rangle \}_{[3]}
\\
|6\rangle \equiv \left|{\bf 1};70\left(1\half(1)\right)J^{-}
 \right\rangle
& = &
|[1^3]^C\rangle \{ |[21]^O \rangle |[1^3]^F \rangle |[21]^S \rangle \}_{[1^3]}~~.
\end{eqnarray}

\noindent{\it c) $N=2$ positive parity baryons}

There are flavor decuplet states with
$J^P=(\FRAC{1}{2}^+)^{2}$, $(\FRAC{3}{2}^+)^{3}$,
$(\FRAC{5}{2}^+)^{2}$, and $\FRAC{7}{2}^+$,
flavor octet states with
 $(\FRAC{1}{2}^+)^{4}$, $(\FRAC{3}{2}^+)^{5}$,
$(\FRAC{5}{2}^+)^{3}$, and $\FRAC{7}{2}^+$,
and flavor singlet states with
 $(\FRAC{1}{2}^+)^{2}$, $(\FRAC{3}{2}^+)^{2}$, and
$(\FRAC{5}{2}^+)^{2}$:
\begin{eqnarray}
|7_L\rangle \equiv \left|{\bf 10};56\left(L\half(3)\right)J^{+}
\right\rangle
& = & |[1^3]^C\rangle  |[3]^O \rangle |[3]^F \rangle |[3]^S \rangle
\\
|8_L\rangle \equiv \left|{\bf 10};70\left(L\half(1)\right)J^{+}
\right\rangle
& = &
|[1^3]^C\rangle  \{ |[21]^O \rangle |[3]^F \rangle |[21]^S \rangle \}_{[3]}
\\
|9_L\rangle \equiv \left|{\bf 8};70\left(L\half(3)\right)J^{+}
\right\rangle
& = &
|[1^3]^C\rangle \{|[21]^O \rangle |[21]^F \rangle \}_{[3]} |[3]^S \rangle
\\
|10_L\rangle \equiv \left|{\bf 8};56\left(L\half(1)\right)J^{+}
\right\rangle
& = &
|[1^3]^C\rangle  |3]^O \rangle \{|[21]^F \rangle |[21]^S \rangle  \}_{[3]}
\\
|11_L\rangle \equiv \left|{\bf 8};70\left(L\half(1)\right)J^{+}
\right\rangle
& = &
|[1^3]^C\rangle \{ |[21]^O \rangle |[21]^F \rangle |[21]^S \rangle \}_{[3]}
\\
|13_L\rangle \equiv \left|{\bf 1};70\left(L\half(1)\right)J^{+}
\right\rangle
& = &
|[1^3]^C\rangle  \{ |[21]^O \rangle |[1^3]^F \rangle |[21]^S \rangle \}_{[1^3]}
\end{eqnarray}
with $L$ = 0 and 2, and
\begin{eqnarray}
|12\rangle \equiv \left|{\bf 8};20\left(1\half(1)\right)J^{+}
\right\rangle
& = &
|[1^3]^C\rangle |1^3]^O \rangle \{|[21]^F \rangle |[21]^S \rangle  \}_{[1^3]}
\\
|14\rangle \equiv \left|{\bf 1};20\left(1\half(3)\right)J^{+}
\right\rangle
& = &
|[1^3]^C\rangle  |[1^3]^O  \rangle  |[1^3]^F \rangle |[3]^S \rangle
\label{eq:44}
\end{eqnarray}
for $L$ = 1.

Here
\begin{eqnarray}
	\{|[21]^\alpha \rangle  |[21]^\beta \rangle\}_{[3]}
	&=& {1\over \sqrt{2} } \left\{
 |[21]^\alpha {\rm {\small MS}} \rangle |[21]^\beta {\rm {\small MS}} \rangle
 +|[21]^\alpha {\tiny  {\rm MA}} \rangle |[21]^\beta {\tiny  {\rm MA}} \rangle
\right\}
\\
	\{|[21]^\alpha \rangle  |[21]^\beta \rangle\}_{[1^3]}
	&=& {1\over \sqrt{2}} \left\{
|[21]^\alpha {\rm {\small MS}} \rangle |[21]^\beta {\tiny  {\rm MA}} \rangle
- |[21]^\alpha {\tiny  {\rm MA}} \rangle |[21]^\beta {\rm {\small MS}} \rangle
\right\}
\\
\{|[21]^\alpha \rangle |[21]^\beta \rangle |[21]^\gamma \rangle\}_{[3]}
		&=& {1\over 2} \left\{
-  |[21]^\alpha {\rm {\small MS}} \rangle |[21]^\beta {\rm {\small MS}} \rangle |[21]^\gamma {\rm {\small MS}} \rangle
+  |[21]^\alpha {\rm {\small MS}} \rangle |[21]^\beta {\tiny  {\rm MA}} \rangle |[21]^\gamma {\tiny  {\rm MA}} \rangle
\right.
\nonumber\\
&+& \left. \!|[21]^\alpha {\tiny  {\rm MA}} \rangle |[21]^\beta {\rm {\small MS}} \rangle |[21]^\gamma
{\tiny  {\rm MA}} \rangle
\!+\!
|[21]^\alpha {\tiny  {\rm MA}} \rangle |[21]^\beta {\tiny  {\rm MA}} \rangle |[21]^\gamma {\rm {\small MS}} \rangle
\right\} ~.
\end{eqnarray}
The orbital wave function in the
coordinate space can be written by Jacobi's coordinates,
$\mbf(\xi) =
(\mbf(r)_1-\mbf(r)_2)/\sqrt{2}$,
$\mbf(\eta) = (\mbf(r)_1+\mbf(r)_2-2\mbf(r)_3)/\sqrt{6}$ and
$\mbf(R)_G=(\mbf(r)_1+\mbf(r)_2+\mbf(r)_3)/\sqrt{3}$.
When we write $ |NL[f]\rangle $, they are
\begin{eqnarray}
|00[3]\rangle & = & \psi_{0s}(\mbf(\xi))\psi_{0s}(\mbf(\eta))
\\
|01[21]{\rm {\small MS}}\rangle & = & \psi_{0s}(\mbf(\xi))\psi_{0p}(\mbf(\eta))
\\
|01[21]{\tiny  {\rm MA}}\rangle & = & \psi_{0p}(\mbf(\xi))\psi_{0s}(\mbf(\eta))
\\
|01[1^{3}]\rangle & = & [\psi_{0p}(\mbf(\xi))
\times \psi_{0p}(\mbf(\eta))]^{1}
\\
|02[3]\rangle & = & {1\over \sqrt{2}}
\{ \psi_{0d}(\mbf(\xi))\psi_{0s}(\mbf(\eta))
+\psi_{0s}(\mbf(\xi))\psi_{0d}(\mbf(\eta)) \}
\\
|02[21]{\rm {\small MS}}\rangle & = & {1\over \sqrt{2}}
\{ \psi_{0d}(\mbf(\xi))\psi_{0s}(\mbf(\eta))
-\psi_{0s}(\mbf(\xi))\psi_{0d}(\mbf(\eta)) \}
\\
|02[21]{\tiny  {\rm MA}}\rangle & = & [ \psi_{0p}(\mbf(\xi))
\times \psi_{0p}(\mbf(\eta))]^{2}
\\
|10[3]\rangle & = & {1\over \sqrt{2}}
\{ \psi_{1s}(\mbf(\xi))\psi_{0s}(\mbf(\eta))
+\psi_{0s}(\mbf(\xi))\psi_{1s}(\mbf(\eta)) \}
\\
|10[21]{\rm {\small MS}}\rangle & = & {1\over \sqrt{2}}
\{ \psi_{1s}(\mbf(\xi))\psi_{0s}(\mbf(\eta))
-\psi_{0s}(\mbf(\xi))\psi_{1s}(\mbf(\eta)) \}
\\
|10[21]{\tiny  {\rm MA}}\rangle & = & [ \psi_{0p}(\mbf(\xi))
\times \psi_{0p}(\mbf(\eta))]^{0} ~~,
\end{eqnarray}
where $[a_{l}\times b_{l'}]^{L}_{M}
= \sum (lml'm'|LM) a_{lm}b_{l'm'}$.

The flavor part is the same as in ref.\ \cite{Is92}.
For the proton, it is
\begin{eqnarray}
    |[3]\rangle	 & = & (duu+udu+uud)
  \\
	|[21]{\rm {\small MS}}\rangle & = & {1\over\sqrt{6}}(-udu-duu+2uud)
  \\
	|[21]{\tiny  {\rm MA}}\rangle & = & {1\over\sqrt{2}}(udu-duu) ~~.
\end{eqnarray}

\subsubsection{Matrix Elements}
The operators we consider can be written as
\begin{eqnarray}
	{\cal O} & = & \sum_{(i<j)} \left\{
	  {\cal O}_c ^{C}  ({\cal S}^F{\cal O}_c^O+{\cal A}^F{{\overline {\cal O}}}_c^O)~1
+ {\cal O}_{ss}^{C}({\cal S}^F{\cal O}_{ss}^O
+{\cal A}^F{{\overline {\cal O}}}_{ss}^O)~\sigma\cdot\sigma
\right.\nonumber\\
&+& \left.
 {\cal O}_{ls}^{C}({\cal S}^F{\cal O}_{ls}^O
 +{\cal A}^F{{\overline {\cal O}}}_{ls}^O)~L\cdot S
+ {\cal O}_{t}^{C}({\cal S}^F{\cal O}_{t}^O
+{\cal A}^F{{\overline {\cal O}}}_{t}^O)~S_{12}\right\}.
\label{eq:symO}
\end{eqnarray}
Then, the matrix element
\begin{eqnarray}
	{\cal O}(n'_{L'},n_{L}) & \equiv &
	 {1\over \sqrt{2J+1}}\langle n'(LS')J || {\cal O} ||n(LS)J \rangle
\end{eqnarray}
 is reduced to sum of the two-body
matrix elements.  Here $n$ is the number expressing the states
defined  by the eqs. (\ref{eq:31}) -- (\ref{eq:44}).

\noindent{\it a) Flavor-decuplet positive parity baryons}

\begin{eqnarray}
{\cal O}(1,1)
& = & A_{0s}+ \Delta_{0s}
\label{eq:mateleS10}\\
{\cal O}(7_0,7_0)
& = &
{1\over 2} \left\{\rule{0pt}{0.5cm}\right. A_{0s}+A_{1s}+\Delta_{0s}+\Delta_{1s}\left.\rule{0pt}{0.5cm}\right\}
\label{eq:matele1S}
\\
{\cal O}(7_{0},7_{2})
& = & {1\over 2}C_{t}(0\half(3)2\half(3)J)\sqrt{5}\;
\theta_{1s-0d}
\\
{\cal O}(7_{0},8_{2})
& = & {1\over2\sqrt{2}} C_{t}(0\half(3)2\half(1)J)\sqrt{10}\;
\theta_{1s-0d}
\\
{\cal O}(8_{0},8_{0})
& = &
{1\over 4} \left\{\rule{0pt}{0.5cm}\right. A_{0s}+A_{1s}+2A_{0p}
+\Delta_{0s}+\Delta_{1s}-6\Delta_{0p}\left.\rule{0pt}{0.5cm}\right\}
\\
{\cal O}(8_{0},7_{2})
& = &
{1\over 2\sqrt{2}} C_{t}(0\half(1)2\half(3)J)(-\sqrt{10})\;
 \theta_{1s-0d}
\\
{\cal O}(7_{2},7_{2})
& = &
{1\over 2} \left\{\rule{0pt}{0.5cm}\right. A_{0s}+A_{0d}+\Delta_{0s}+\Delta_{0d}
\nonumber\\
&+& C_{ls}(2\half(3)2\half(3)J)(-\sqrt{3\over 2})\;
\chi_{0d}
+ C_{t}(2\half(3)2\half(3)J)(-\sqrt{10\over 7})\;
\theta_{0d}\left.\rule{0pt}{0.5cm}\right\}
\\
{\cal O}(7_{2},8_{2}) &=&
{1\over 2\sqrt{2}}\left\{\rule{0pt}{0.5cm}\right.
 C_{ls}(2\half(3)2\half(1)J)(-\sqrt{3\over 5})\;
 \chi_{0d}
+C_{t}(2\half(3)2\half(1)J)(-\sqrt{20\over 7})\;
\theta_{0d}\left.\rule{0pt}{0.5cm}\right\}
\\
{\cal O}(8_{2},8_{2})
& = &
{1\over 4} \left\{\rule{0pt}{0.5cm}\right. A_{0s}+A_{0d}+2A_{0p}
+\Delta_{0s}+\Delta_{0d}-6\Delta_{0p}
\nonumber\\
&+& C_{ls}(2\half(1)2\half(1)J)(-\sqrt{12\over 5})\;
 \chi_{0d}\left.\rule{0pt}{0.5cm}\right\}
\\
\end{eqnarray}

\noindent{\it b) Flavor-octet positive parity baryons}

\begin{eqnarray}
{\cal O}(2,2)
& = & {1\over2} \left\{\rule{0pt}{0.5cm}\right. A_{0s}+ \Delta_{0s}+{\overline A}_{0s}
-3{\overline \Delta}_{0s}\left.\rule{0pt}{0.5cm}\right\}
\\
{\cal O}(9_{0},9_{0})
& = &
{1\over 4} \left\{\rule{0pt}{0.5cm}\right. A_{0s}+A_{1s}+2 {\overline A}_{0p}
+\Delta_{0s}+\Delta_{1s}+2{\overline \Delta}_{0p}\left.\rule{0pt}{0.5cm}\right\}
\\
{\cal O}(9_{0},12)
& = & -{1\over 2} C_{ls}(0\half(3)1\half(1)J)
\sqrt{1\over 3}\;{\overline \chi}_{0p}
\\
{\cal O}(9_{0},9_{2})
& = &
{1\over 4}
 C_{t}(0\half(3)2\half(3)J)\left\{\rule{0pt}{0.5cm}\right. (-\sqrt{2})2\;{\overline \theta}_{0p}
+\sqrt{5}\; \theta_{1s-0d}\left.\rule{0pt}{0.5cm}\right\}
\\
{\cal O}(9_{0},10_{2})
& = &
{1\over 4}
 C_{t}(0\half(3)2\half(1)J)\sqrt{10}\; \theta_{1s-0d}
\\
{\cal O}(9_{0},11_{2})
& = &
{1\over 4\sqrt{2}}
 C_{t}(0\half(3)2\half(1)J)\left\{\rule{0pt}{0.5cm}\right. (-\sqrt{4})2 \;{\overline \theta}_{0p}
-\sqrt{10} \; \theta_{1s-0d}\left.\rule{0pt}{0.5cm}\right\}
\\
{\cal O}(10_{0},10_{0})
& = &
{1\over 4}
\left\{\rule{0pt}{0.5cm}\right. A_{0s}+A_{1s}+{\overline A}_{0s}+{\overline A}_{1s}
+\Delta_{0s}+\Delta_{1s}-3{\overline \Delta}_{0s}-3{\overline \Delta}_{1s}\left.\rule{0pt}{0.5cm}\right\}
\\
{\cal O}(10_{0},11_{0})
& = &
{1\over 4\sqrt{2}}
\left\{\rule{0pt}{0.5cm}\right. A_{0s}-A_{1s}-{\overline A}_{0s}+{\overline A}_{1s}+
\Delta_{0s}-\Delta_{1s}+3{\overline \Delta}_{0s}-3{\overline \Delta}_{1s}\left.\rule{0pt}{0.5cm}\right\}
\\
{\cal O}(10_{0},9_{2})
& = &
{1\over 4}
 C_{t}(0\half(1)2\half(3)J)(-\sqrt{10})\; \theta_{1s-0d}
\\
{\cal O}(11_{0},11_{0})
& = &
{1\over 8}
\left\{\rule{0pt}{0.5cm}\right. A_{0s}+A_{1s}+2A_{0p}+{\overline A}_{0s}+{\overline A}_{1s}+2{\overline A}_{0p}
\nonumber\\
&&+\Delta_{0s}+\Delta_{1s}-6\Delta_{0p}-3{\overline \Delta}_{0s}-3{\overline \Delta}_{1s}
+2{\overline \Delta}_{0p}\left.\rule{0pt}{0.5cm}\right\}
\\
{\cal O}(11_{0},12)
& = &
-{1\over 2\sqrt{2}}
 C_{ls}(0\half(1)1\half(1)J)\sqrt{4\over 3}\;{\overline \chi}_{0p}
\\
{\cal O}(11_{0},9_{2})
& = &
{1\over 4\sqrt{2}}
C_{t}(0\half(1)2\half(3)J)\left\{\rule{0pt}{0.5cm}\right. \sqrt{4}\: 2 \;{\overline \theta}_{0p}
 -(-\sqrt{10})\;{\overline \theta}_{1s-0d}\left.\rule{0pt}{0.5cm}\right\}
\\
{\cal O}(9_{2},9_{2})
& = &
{1\over 4} \left\{\rule{0pt}{0.5cm}\right. A_{0s}+A_{0d}+2 {\overline A}_{0p}+\Delta_{0s}+\Delta_{0d}
+2{\overline \Delta}_{0p}
\nonumber\\
&+& C_{ls}(2\half(3)2\half(3)J)((-\sqrt{3\over8})2\;{\overline \chi}_{0p}
+(-\sqrt{3\over2})\; \chi_{0d})
\nonumber\\
&+&C_{t}(2\half(3)2\half(3)J)((-\sqrt{7\over 10})2\;{\overline \theta}_{0p}
+(-\sqrt{10\over7})\; \theta_{0d})
\left.\rule{0pt}{0.5cm}\right\}
\\
{\cal O}(9_2,10_2) &=&
{1\over 4}  \left\{\rule{0pt}{0.5cm}\right. C_{ls}(2\half(3)2\half(1)J)(-\sqrt{3\over 5})\;
 \chi_{0d}
+C_{t}(2\half(3)2\half(1)J)(-\sqrt{20\over 7})\; \theta_{0d}
\left.\rule{0pt}{0.5cm}\right\}
\\
{\cal O}(9_2,11_2) &=&
{1\over 4\sqrt{2}} \left\{\rule{0pt}{0.5cm}\right. C_{ls}(2\half(3)2\half(1)J)
((-\sqrt{3\over 20})2\;{\overline \chi}_{0p}-(-\sqrt{3\over 5})\;
 \chi_{0d})
\nonumber\\
&+&C_{t}(2\half(3)2\half(1)J)((-\sqrt{7\over 5})2
\;{\overline \theta}_{0p}-(-\sqrt{20\over 7})\; \theta_{0d})\left.\rule{0pt}{0.5cm}\right\}
\\
{\cal O}(9_2,12) &=&
-{1\over 2}  \left\{\rule{0pt}{0.5cm}\right. C_{ls}(2\half(3)1\half(1)J)
(-\sqrt{1\over 12})\;{\overline \chi}_{0p}
+C_{t}(2\half(3)1\half(1)J) (-\sqrt{3})\;{\overline \theta}_{0p}\left.\rule{0pt}{0.5cm}\right\}
\\
{\cal O}(10_2,10_2)
& = &
{1\over 4}
\left\{\rule{0pt}{0.5cm}\right. A_{0s}+A_{0d}+{\overline A}_{0s}+{\overline A}_{0d}+\Delta_{0s}
+\Delta_{0d}-3{\overline \Delta}_{0s}-3{\overline \Delta}_{0d}
\nonumber\\
&+& C_{ls}(2\half(1)2\half(1)J)(-\sqrt{12\over 5})\;
 \chi_{0d}\left.\rule{0pt}{0.5cm}\right\}
\\
{\cal O}(10_2,11_2)
& = &
{1\over 4\sqrt{2}}
\left\{\rule{0pt}{0.5cm}\right. A_{0s}-A_{0d}-{\overline A}_{0s}+{\overline A}_{0d}+
\Delta_{0s}-\Delta_{0d}+3{\overline \Delta}_{0s}-3{\overline \Delta}_{0d}
\nonumber\\
&-&  C_{ls}(2\half(1)2\half(1)J)(-\sqrt{12\over 5})\;
\chi_{0d}\left.\rule{0pt}{0.5cm}\right\}
\\
{\cal O}(11_2,11_2)
& = &
{1\over 8}
\left\{\rule{0pt}{0.5cm}\right. A_{0s}+A_{0d}+2A_{0p}+{\overline A}_{0s}+{\overline A}_{0d}+2{\overline A}_{0p}
\nonumber\\
&&~~ + \Delta_{0s}+\Delta_{0d}-6\Delta_{0p}-3{\overline \Delta}_{0s}-3{\overline \Delta}_{0d}
+2{\overline \Delta}_{0p}
\nonumber\\
&+& C_{ls}(2\half(1)2\half(1)J) ((-\sqrt{3\over 5})2\;{\overline \chi}_{0p})
+(-\sqrt{12\over 5})\; \chi_{0d}\left.\rule{0pt}{0.5cm}\right\}
\\
{\cal O}(11_2,12) &=& -{1\over 2\sqrt{2}}
C_{ls}(2\half(1)1\half(1)J) (-\sqrt{1\over 3})\;{\overline \chi}_{0p}
\\
{\cal O}(12,12)
& = &
{1\over 2} \left\{\rule{0pt}{0.5cm}\right. A_{0p}+{\overline A}_{0p}-3\Delta_{0p}+{\overline \Delta}_{0p}
+ C_{ls}(1\half(1)1\half(1)J)(-\sqrt{1\over 3})\;{\overline \chi}_{0p}\left.\rule{0pt}{0.5cm}\right\}
\\
\end{eqnarray}

\noindent{\it c) Flavor-singlet positive parity baryons}

\begin{eqnarray}
{\cal O}(13_{0},13_{0}) & = &{1\over 4} \left\{\rule{0pt}{0.5cm}\right. 2{\overline A}_{0p}+{\overline A}_{0s}
+{\overline A}_{1s}+2{\overline \Delta}_{0p}
-3{\overline \Delta}_{0s}-3{\overline \Delta}_{1s}\left.\rule{0pt}{0.5cm}\right\}
	\\
{\cal O}(13_{0},14) &=& -{1\over\sqrt{2}}
 C_{ls}(0\half(1)1\half(3)J)(-\sqrt{1\over 3})\;{\overline \chi}_{0p}
\\
{\cal O}(13_{2},13_{2}) & = &{1\over 4} \left\{\rule{0pt}{0.5cm}\right. 2{\overline A}_{0p}+{\overline A}_{0s}
+{\overline A}_{0d}+2{\overline \Delta}_{0p}
-3{\overline \Delta}_{0s}-3{\overline \Delta}_{0d}
\nonumber\\
&+& C_{ls}(2\half(1)2\half(1)J)(-\sqrt{3\over 5})2\;{\overline \chi}_{0p}
\left.\rule{0pt}{0.5cm}\right\}
	\\
{\cal O}(13_{2},14) &=& -{1\over\sqrt{2}}\left\{\rule{0pt}{0.5cm}\right.
 C_{ls}(2\half(1)1\half(3)J)\sqrt{1\over 12}\;{\overline \chi}_{0p}
+C_{t}(2\half(1)1\half(3)J)\sqrt{3}\;{\overline \theta}_{0p}
 \left.\rule{0pt}{0.5cm}\right\}
\\
{\cal O}(14,14) & = & {\overline A}_{0p}+{\overline \Delta}_{0p}
\nonumber\\
&+& C_{ls}(1\half(3)1\half(3)J)(-\sqrt{5\over 24})\;{\overline \chi}_{0p}
+ C_{t}(1\half(3)1\half(3)J)\sqrt{5\over 6}\;{\overline \theta}_{0p}
\end{eqnarray}

\noindent{\it d) Negative parity baryons}

\begin{eqnarray}
{\cal O}(3,3)
& = &{1\over2} \left\{\rule{0pt}{0.5cm}\right. A_{0s}+A_{0p}+ \Delta_{0s}-3 \Delta_{0p}\left.\rule{0pt}{0.5cm}\right\}
\label{eq:mateleP10}\\
{\cal O}(4,4)
& = &{1\over2} \left\{\rule{0pt}{0.5cm}\right. A_{0s}+\Delta_{0s}+{\overline A}_{0p}+{\overline \Delta}_{0p}
\nonumber\\
&+& C_{ls}(1\half(3)1\half(3)J)(-\sqrt{5\over 6})\;{\overline \chi}_{0p}
+ C_{t}(1\half(3)1\half(3)J)(-\sqrt{10\over 3}){\;{\overline \theta}}_{0p}
\left.\rule{0pt}{0.5cm}\right\}
	\\
{\cal O}(4,5)
& = & {1\over 2\sqrt{2}}\left\{\rule{0pt}{0.5cm}\right. C_{ls}(1\half(3)1\half(1)J)
 (-\sqrt{1\over 3}) \;{\overline \chi}_{0p}
+ C_{t}(1\half(3)1\half(1)J) (-\sqrt{20\over 3}) {\;{\overline \theta}}_{0p}
\left.\rule{0pt}{0.5cm}\right\}
\\
{\cal O}(5,5)
& = &{1\over 4} \left\{\rule{0pt}{0.5cm}\right.
A_{0s}+A_{0p} +\Delta_{0s}-3\Delta_{0p}+{\overline A}_{0s}+{\overline A}_{0p}
-3{\overline \Delta}_{0s}+{\overline \Delta}_{0p}
\nonumber\\
&+& C_{ls}(1\half(1)1\half(1)J) (-\sqrt{4\over 3}) \;{\overline \chi}_{0p}
\left.\rule{0pt}{0.5cm}\right\}
\\
{\cal O}(6,6)
& = &{1\over2} \left\{\rule{0pt}{0.5cm}\right. {\overline A}_{0s}+{\overline A}_{0p}-3{\overline \Delta}_{0s}
+{\overline \Delta}_{0p}
+ C_{ls}(1\half(1)1\half(1)J) (-\sqrt{4\over 3}) \;{\overline \chi}_{0p}
\left.\rule{0pt}{0.5cm}\right\} ~~.
\label{eq:mateleP1}
\end{eqnarray}
$C_{ls}(L'S'LSJ)$ and $C_t(L'S'LSJ)$ are defined as
\begin{eqnarray}
	C_{\alpha}(L'S'LSJ) & = &
	 \sqrt{(2J+1)(2L'+1)(2L+1)(2S'+1)(2S+1)}
	\ninej(L',S',J,\lambda,\lambda,0,L,S,J)
\end{eqnarray}
with $\lambda$ = 1 and 2 for $\alpha$ = {\it ls} and {\it t},
 respectively.
The radial integrations are:
\begin{eqnarray}
	A_{nl} & = & 3\langle nl|{{\cal O}_c^O}_{(ij)=(12)}
	|nl\rangle \langle {{\cal O}_{c}^{C}}_{(ij)=(12)} \rangle
{} \\
	\Delta_{nl} & = & 3\langle nl|{{\cal O}_{ss}^O}_{12}
	|nl\rangle \langle {\cal O}_{ss}^{C} \rangle
{} \\
	\chi_{nl} & = &3 \langle nl|{{\cal O}_{ls}^O}_{12}
	|nl\rangle \langle {\cal O}_{ls}^{C} \rangle
{} \\
	\theta_{nl} & = & 3\langle nl|{{\cal O}_{t}^O}_{12}
	|nl\rangle \langle {\cal O}_{t}^{C} \rangle
{} \\
	\theta_{n'l'-nl} & = & 3\langle n'l'|{{\cal O}_{t}^O}_{12}
	|nl\rangle \langle {\cal O}_{t}^{C} \rangle ~~.
{}
\end{eqnarray}
Those with bars are similarly defined.
{}From eqs.(\ref{eq:mateleS10})--(\ref{eq:mateleP1}),
one can actually see
only the flavor-antisymmetric $0p$ pairs
and the flavor-symmetric $0d$ pairs are relevant
for the noncentral
part in the single baryons.

 For OGE, the terms in  eq.\ (\ref{eq:symO}) are
	\begin{eqnarray}
	{\cal O}^O_{ss} = {\overline {\cal O}}^O_{ss} & = &
	 - 4\pi\alpha_s {1\over 6m^2} \delta(\mbf(r))
		  \\
	{\cal O}^O_{ls} = {\overline {\cal O}}^O_{ls} & = &
	 - 4\pi\alpha_s {3\over 2m^2}{1\over 4\pi r^3}
		  \\
	{\cal O}^O_{t} = {\overline {\cal O}}^O_{t} & = &
	- 4\pi\alpha_s {1\over 4m^2}{1\over 4\pi r^3}
	\end{eqnarray}
with
$$
{\cal O}^C_\alpha = {\lambda\cdot\lambda \over 4}.
$$
Therefore, the two-body matrix elements become:
\begin{eqnarray}
	\Delta_{0s} = {\overline \Delta}_{0s} & = & {1\over 2}\mu_{\rm OGE}
\\
	\Delta_{1s} = {\overline \Delta}_{1s} & = & {3\over 4}\mu_{\rm OGE}
\\
	\Delta_{nl} = {\overline \Delta}_{nl} & = & 0 ~~(l>0)
\\
	\;{\overline \chi}_{0p} & = & {3\over 2}\mu_{\rm OGE}
\label{eq:barchi0pOGE}
\\
	\chi_{0d} & = & {3\over 5}\mu_{\rm OGE}
\\
	\;{\overline \theta}_{0p} & = &  {1\over 4}\mu_{\rm OGE}
\label{eq:bartheta0pOGE}
\\
	\theta_{0d} & = &  {1\over 10}\mu_{\rm OGE}
\\
	\theta_{0d-1s} & = &  \sqrt{1\over 160}\mu_{\rm OGE}
\end{eqnarray}
with
$$
\mu_{\rm OGE} =
\half(1) (A_{0s}+\Delta_{0s}-{\overline A}_{0s}+3{\overline \Delta}_{0s})=
 \alpha_s {4\over 3} {1\over\sqrt{2\pi}} {1\over m^2b^3},
$$
which corresponds to the $S$-wave N-$\Delta$ mass difference
(= 293 MeV).

As for \mbox{\rm I\thinspace I\thinspace I}, all operators without a bar vanish.  The
flavor-singlet operators are
	\begin{eqnarray}
	{\overline {\cal O}}^O_{ss} & = &
	 - V_{0}^{(2)} {3\over 16} \delta(\mbf(r))
		  \\
	{\overline {\cal O}}^O_{ls} & = &
	 V_{0}^{(2)}  {9\over 4m^2} {\delta(r) \over 4\pi r^{4}}
		  \\
	{\overline {\cal O}}^O_{t} & = &
	  V_{0}^{(2)}  {5\over 4m^2} {\delta(r) \over 4\pi r^{4}}
	\end{eqnarray}
with
\begin{eqnarray}
{\cal O}^C_{ss} =
{\cal O}^C_{ls} &=& 1 \\
{\cal O}^C_t &=& 1 - {3\over4}{\lambda\cdot\lambda \over 4} ~~.
\end{eqnarray}
Thus we obtain the two-body matrix elements for \mbox{\rm I\thinspace I\thinspace I}\ as
\begin{eqnarray}
	{\overline \Delta}_{0s} & = & {1\over 4}\mu_{\rm III}
\\
	{\overline \Delta}_{1s} & = & {3\over 8}\mu_{\rm III}
\\
	 {\overline \Delta}_{nl} & = & 0 ~~(l>0)
\\
	\;{\overline \chi}_{0p} & = & -{1\over m^{2}b^{2}} \mu_{\rm III}
\label{eq:barchi0pIII}
\\
	\;{\overline \chi}_{nl} & = & 0 ~~(l>1)
\\
	\;{\overline \theta}_{0p} & = &  -{5\over 6}{1\over m^{2}b^{2}} \mu_{\rm III}
\label{eq:bartheta0pIII}
\\
\;{\overline \theta}_{nl} & = &  0 ~~(l>2)
\end{eqnarray}
with
$$
\mu_{\rm III} =
- {9\over 4}  V_{0}^{(2)} {1\over\sqrt{2\pi b^{2}}^{3}} ~~.
$$

The mass of baryons are obtained from
eq.(\ref{eq:mateleS10})-(\ref{eq:mateleP1}),
 by diagonarizing them if
necessary, and adding the central part.
\subsection{Two Nucleons}

Here we consider a six-quark system $(0s)^{5}(0p)$,
with quantum number of
two nucleons with relative partial $P$-wave.
 The wave function is
\begin{equation}
	\Psi = {\cal A}_{q}\Phi \equiv
	{\cal A}_{q}\{\phi^{2}_{N}\psi_{0p}(R)\}	 ~~,
\end{equation}
where ${\cal A}_{q}$ is an antisymmetrizer with respect
to all six quarks,
$\phi_{N}$ is the nucleon wave function defined
by the previous section,
and the $\psi_{0p}(R)$ is a $P$-wave harmonic oscillator
with size parameter
$b$ and $R=(r_{1}+r_{2}+r_{3}-r_{4}-r_{5}-r_{6})/\sqrt{6}$.

Noncentral operators relevant to this state
are orbitally-antisymmetric two terms in eq.(\ref{eq:projop}).
The expectation value by the above
state can written as

\begin{eqnarray}
	\langle \Psi |{\cal O} | \Psi\rangle & = &
\langle \Phi |\sum_{i<j}({\overline {\cal O}}^A_{ij} + {\cal O}^S_{ij}
){\cal A}_{q}|\Phi\rangle
/
\langle \Phi |{\cal A}_{q}|\Phi\rangle
 \\
	 & = &
\langle \Phi |\sum_{i<j}({\overline {\cal O}}^A_{ij} +
{\cal O}^S_{ij})(1-9P_{36})|\Phi\rangle
/
\langle \Phi |(1-9P_{36})|\Phi\rangle  ~~,
\label{eq:143}
\end{eqnarray}
where $P_{36}\equiv P_{36}^{c}P_{36}^{f}P_{36}^{s}P_{36}^{o}$
is the exchange operator for quark $i$, and $j$ in the color,
flavor,
spin and orbital space.
The numerator is
\begin{eqnarray}
&   & 	9\langle \Phi| ({\overline {\cal O}}^A_{36} + {\cal O}^S_{36})
 |\Phi\rangle
-	9\left\{\rule{0pt}{0.5cm}\right. 4 \langle \Phi| ({\overline {\cal O}}^A_{14} + {\cal O}^S_{14})P_{36}
|\Phi\rangle
+ \langle \Phi | ({\overline {\cal O}}^A_{36} + {\cal O}^S_{36})P_{36}
 |\Phi\rangle \left.\rule{0pt}{0.5cm}\right\}
\nonumber\\
& = & 	9\left\{\rule{0pt}{0.5cm}\right. 2\langle\Phi| ({\overline {\cal O}}^A_{36} + {\cal O}^S_{36})
|\Phi\rangle
- 	4 \langle \Phi | ({\overline {\cal O}}^A_{14} + {\cal O}^S_{14})P_{36}
|\Phi\rangle\left.\rule{0pt}{0.5cm}\right\}
\nonumber\\
& = & 	18\left\{\rule{0pt}{0.5cm}\right. \langle \Phi|{\overline {\cal O}}^A_{36}|\Phi\rangle
+\langle \Phi |{\cal O}^S_{36}|\Phi\rangle - 2\langle \Phi|{\cal O}^S_{14}P_{36
}|\Phi\rangle\left.\rule{0pt}{0.5cm}\right\}
\label{eq:2Nmatele}
\end{eqnarray}
Here we use
\begin{eqnarray}
	{\cal O}_{16}P_{36} & = & P_{36}{\cal O}_{13}
\\
	\langle\Phi|{\cal O}_{13}|\Phi\rangle & = & \langle\Phi|{\cal O}_{13} P_{36}
	|\Phi\rangle = 0
\\
	\langle\Phi|{\cal O}_{36} P_{36}|\Phi\rangle & = & -\langle\Phi|{\cal O}_{36}
	|\Phi\rangle ~~.
\end{eqnarray}
For the spin-orbit part,
 ${\cal O}_{ij} = f(r_{ij})L_{ij}\cdot S_{ij}$,
 each term in eq.(\ref{eq:2Nmatele}) can be evaluated as
\begin{eqnarray}
	\langle \Phi | {\cal O}_{36} | \Phi\rangle & = & {1\over16}\langle
 f(r_{36})L_{36}\cdot S_{36}(1\mp P_{36}^{c})
 (1\mp P_{36}^{f})(1+P_{36}^{s})(1-P_{36}^{o}) \rangle
	  \\
	 & = & {1\over 2}(1\mp \langle P_{36}^{c}\rangle)
	  {1\over 2}(\langle f(r_{36})L_{36} (1\!-\!P_{36}^{o}) \rangle)
	 {1\over 4}\langle S_{36}(1+\!P_{36}^{s}\mp \! P_{36}^{f}
	 \mp \! P_{36}^{sf}) \rangle
	  \\
	\langle \Phi | {\cal O}_{14}P_{36} | \Phi\rangle & = &
	{1\over16}\langle
 f(r_{14})L_{14}\cdot S_{14}(1\mp P_{14}^{c})(1\mp P_{14}^{f})
 (1+P_{14}^{s})(1-P_{14}^{o})P_{36} \rangle
	  \\
	 & = & {1\over 2}(\langle P_{36}^{c}\rangle\mp\langle
	  P_{14}^{c}P_{36}^{c}\rangle)
	 {1\over 2}(\langle f(r_{14})L_{14}(1-P_{14}^{o})P_{36}^{o} \rangle)
	  \nonumber\\&&
\times {1\over 4}\langle S_{14}(1+P_{14}^{s}\mp P_{14}^{f}
\mp P_{14}^{sf})P_{36}^{sf}\rangle ~~.
\end{eqnarray}
The $\mp$ reads $-$ for ${\overline {\cal O}}^{A}$ and $+$ for ${\cal O}^{S}$.
The color part is  $\langle P_{36}^{c}\rangle = \langle P_{14}^{c}P_{36}^{c}
\rangle = {1\over3}$.
The spin-flavor part can be calculated directly:
\begin{eqnarray}
	\langle p^\uparrow p^\uparrow | S_{36}(1+P_{36}^{s}\mp P_{36}^{f}
	\mp P_{36}^{sf}) |p^\uparrow p^\uparrow\rangle & = &
	{1\over4}\left\{\rule{0pt}{0.5cm}\right. {1\over3}+{1\over3}\mp{7\over27}\mp{7\over27}
	\left.\rule{0pt}{0.5cm}\right\} = \left\{ \matrix{ {1\over27} \cr {8\over27}}\right.
	  \\
	\langle p^\uparrow p^\uparrow | S_{14}(1+P_{14}^{s}\mp P_{14}^{f}
	\mp P_{14}^{sf})  P_{36}^{sf} |p^\uparrow p^\uparrow\rangle & = &
	{1\over4}\left\{\rule{0pt}{0.5cm}\right. {5\over81}+{5\over81}\mp{5\over81}\mp{5\over81}
	\left.\rule{0pt}{0.5cm}\right\} = \left\{\matrix{ 0 \cr {5\over81}}\right. .
\end{eqnarray}
$\langle f(r_{ij})L_{ij}(1-P_{36}^{o}) \rangle = {2 \over 9}
\;{\overline \chi}^{A}_{0p}$ (or ${2 \over 9} \chi^{S}_{0p}$)
for ${\overline {\cal O}}^{A}$ (or ${\cal O}^{S}$) and
$\langle f(r_{ij})L_{ij}(1-P_{36}^{o}) \rangle = {2 \over 9}
\chi^{S}_{0p}$.

The denominator of eq.(\ref{eq:143}) is ${50\over 81}$
\cite{MYO84,TSY89}.  Thus
the matrix element eq.(\ref{eq:2Nmatele}) is
\begin{eqnarray}
		\langle \Psi |{\cal O} | \Psi\rangle  & = & {3 \over 75}
		\;{\overline \chi}^{A}_{0p} + {38\over75}\chi^{S}_{0p}.
	\\
\end{eqnarray}
The coefficients are listed as $C_{NN}$ in Table 2.
The tensor part can similarly be obtained:
\begin{eqnarray}
		\langle \Psi |{\cal O} | \Psi\rangle  & = & -{4 \over 75}
		\;{\overline \theta}^{A}_{0p} + {21\over75}\theta^{S}_{0p} \\
\end{eqnarray}
by using
\begin{eqnarray}
	\langle p^\uparrow p^\uparrow | \sigma^{+}_{3}\sigma^{+}_{6}
	(1+P_{36}^{s}\mp P_{36}^{f}\mp P_{36}^{sf})
	|p^\downarrow p^\downarrow\rangle & = &
	{1\over4}\left\{\rule{0pt}{0.5cm}\right. {9\over81}+{9\over81}\mp{17\over81}
	\mp{17\over81}\left.\rule{0pt}{0.5cm}\right\} = \left\{ \matrix{ -{4\over81}
	\cr {13\over81}}\right.
	  \\
	\langle p^\uparrow p^\uparrow | \sigma^{+}_{1}\sigma^{+}_{4}
	(1+P_{14}^{s}\mp P_{14}^{f}\mp P_{14}^{sf})  P_{36}^{sf}
	|p^\downarrow p^\downarrow\rangle & = &
	{1\over4}\left\{\rule{0pt}{0.5cm}\right. \!{5\over162}\!+\!{5\over162}\!\mp\!
	{5\over162}\!\mp\!{5\over162}\!\left.\rule{0pt}{0.5cm}\right\} =
	\left\{\matrix{ 0 \cr \!{5\over162}}\right. .
\end{eqnarray}
One can clearly see that the flavor symmetric part of the operator
 is dominant in this state
both for the spin-orbit term and the tensor term.

The actual value is obtained by substituting $\chi^{A}_{0p}$
 by $\;{\overline \chi}_{0p}$
 in eqs.(\ref{eq:barchi0pOGE}) and (\ref{eq:barchi0pIII})
and $\;{\overline \chi}^{S}_{0p}$ by $-{3\over4}\mu_{\rm OGE}$,
and by substituting $\;{\overline \theta}^{A}_{0p}$ by $\;{\overline \theta}_{0p}$
in eqs.(\ref{eq:bartheta0pOGE}) and (\ref{eq:bartheta0pIII})
and $\theta^{S}_{0p}$ by $-{1\over8}\mu_{\rm OGE}$.

\newpage

redpajama_set_name: RedPajamaArXiv


1. Covering Letter : One of the authors could be identified as the corresponding author of the paper, who would be responsible for the correspondence with the Editor - in - Chief.
2. Manuscript : Manuscripts can be submitted in a CD (Compact Disc) in MS Word (in addition to one hard copy). Typescript should be sent to the Editor - in - Chief on one side of a good quality bond paper (21.0 x 29.7cms). Pages should be numbered consecutively and the contents arranged in the following order - Title; Name(s) of the author(s); Department(s) and Institution(s); Abstract; Key words; Introduction; Material & Methods; Results; Discussion; Acknowledgment; and reference. Abstract, Tables and Legends for Figures should be typed on separate sheets and not in continuation of the main text.
Title : Title of the article should be short, continuous (broken or hyphenated titles are not acceptable) and yet sufficiently descriptive and informative so as to be useful in indexing and information retrieval.
Abstract : Abstract should be brief (250 words) and indicate the scope and significant results of the paper. It should only highlight the principal findings and conclusions so that it can be used by abstracting services without modification. Conclusions and recommendations not found in the text of the articles should not be inserted in the Abstract. A set of suitable key words arranged alphabetically may be provided.
Introduction : Introduction should be brief and state precisely the scope of the paper. Review of the literature should be restricted to reasons for undertaking the present study and provide only the most essential background. This should cover the study area, study population, sample size, sampling techniques and the data collection techniques and tools, data analyses and statistical analyses.
Results : Only such data are essential for understanding the discussion and main conclusions emerging from the study should be included. The data should be arranged in unified and coherent sequence. Data presented in tables and figures should not be repeated in the text. Only important observations need to be emphasized or summarized.
Discussion : The discussion should deal with the interpretation of results without repeating information already presented under Results. It should relate new findings to the known ones and include logical deductions. It should also mention any weaknesses of the study. The conclusions can be linked with the goals of the study. All hypotheses should, if warranted, clearly be identified as such; recommendations may be included as part of Discussion, only when considered absolutely necessary and relevant.
References : The total number of References should normally be restricted to a maximum of 30.
References to literature cited should be numbered consecutively and placed at the end of the manuscript. In the text they should be indicated above the line (superior). As far as possible mentioning name of author(s) under references should be avoided in text. These should be written in Vancouver style.
1. Standard journal article – Sharma A.K. Singh S, Organ transplantation in HIV infected patients. N. Engl.J. Med. 2002; 347: 284-7.
2. Books and monograph-Murray RR, Rusenthal KS Medical Microbiology, 4th ed. St. Lovis: Mosby; 2002.
3.	Chapter in a book-Meltzen PS, Trent JM. Chromosome alternations in human solid tumors. In: Vogelstein B, editor. The Genetic basis of human cancer, Newyork: MC GrawHill; 2002 p. 93-113.
4.	Conference proceedings-Handen P, Jones WD, Editors. Germ cell Tumors. Proceedings of the 5th Germ cell tumor conference; 2001 Sept 13-15; Leads, U/C Newyork: Springer; 2002.
5.	Dissertation-Singh AK. Prevalence of hypertension in school children. Maulana Azad Medical College; 2003.
6.	Internet article - Abood S. Quality improvement initiatives in running home Am J Nurs, 2002 Jun: 102 (6), available for http/222.muningworld.org/AJN/2002. nurseswatch.com.


text:
Semiconductors Break Out
05/07/07 03:29:08 PM
After slipping into a sideways consolidation in the autumn of 2006, semiconductor stocks broke out in the spring of 2007.
Security: $SOX, SMH
Seasonally speaking, semiconductors tend to outperform from October to December — at least per the research of Yale and Jeff Hirsch in their Stock Traders Almanac. I've heard this notion of semiconductor seasonality before, most recently from Jim Cramer of Mad Money fame, who quipped, "Avoid chip stocks during the summer."
FIGURE 1: PHILADELPHIA SEMICONDUCTOR INDEX, WEEKLY. The consolidation in the $SOX developed after a strong rally from the summer 2006 lows. Insofar as consolidations in trends tend to lead to more trend, the breakout to the upside in the spring of 2007 was little surprise.
Graphic provided by: Prophet Financial, Inc.
Much recent action in the semiconductor indexes and proxies ($SOX and SMH, respectively) seems to support these opinions. In 2004, the SMH (semiconductor HOLDRS) bottomed in August near 28 and by late November were trading north of 34. In 2005, the SMH bottomed in October near 33 and by the first week of January the following year was trading as high as 40.
The year 2006 saw another summer bottom in semiconductor stocks in mid-July near 29 produce a strong rally into October (the SMH topped near 36). But from October to December there was little if any appreciation for semiconductor stocks. Instead, semiconductor stocks moved sideways for week after week throughout the first quarter of 2007 and into the second.
FIGURE 2: SEMICONDUCTOR HOLDRS TRUST, WEEKLY. Alternating Aprils have proved timely buying and selling opportunities for semiconductor stocks over the past few years. As such, the April of 2007 is scheduled to be a buying opportunity.
April has brought alternating fortunes to semiconductor stocks over the past few years. The spring of 2004 was a selling opportunity. The spring of 2005 proved to be an apt time to buy. The spring of 2006 was once again a time to sell. And so it is that the spring of 2007 seems to present another opportunity for speculators to purchase semiconductor stocks at consolidation or depressed prices (see Figures 1 and 2).
The width of the consolidation in the SMH — approximately three points from 33 to 36 — suggests an upside minimum move to the 39 area. As for the $SOX, a 30-point wide consolidation between, roughly, 460 and 490 projects an upside to 520. In both the SMH and the $SOX, these upside projections point to a test of the April highs from 2006 initially (approximately 39 and 535, respectively) and beyond that, perhaps a run at the 2006 highs (approximately 40.5 and 560) as well.
Date:�05/07/07Rank:�2Comment:�

redpajama_set_name: RedPajamaCommonCrawl


This document has been developed and written by the Pressure Equipment Consultation Forum (PECF), Safety Assessment Federation (SAFed) and EEMUA in consultation with other stakeholders within the pressure equipment industry to help those parties involved in the creation of pressure equipment assemblies to ensure that global conformity assessment can be successfully applied. The UK Health and Safety Executive (HSE), which was also involved in producing this publication, supports the guidance as a sensible and proportionate approach to managing health and safety.
The Pressure Equipment Directive (PED) requires that individual items of pressure equipment undergo conformity assessment where appropriate. This also applies to assemblies of pressure equipment which need to undergo global conformity assessment and CE marking. Experience within the UK indicates that generally this process works well when assemblies are placed on the market as complete, factory supplied products. However, when assemblies are created on site at the place of installation the legal process of global conformity assessment is often found to be non-compliant. The document is intended to provide the necessary guidance to all parties with responsibilities for the pressure equipment assembly to ensure global conformity assessment can take place.
The guidance applies to the following directives: Pressure Equipment Directive (97/23/EC), as implemented by the Pressure Equipment Regulations (PER) 1999; and Pressure Equipment Directive (2014/68/EU), as implemented by the Pressure Equipment (Safety) Regulations (PESR) 2016.
This publication is aimed at all parties (other than notified bodies or user inspectorates) who are involved in the design and manufacturer of site installed assemblies in the UK. This includes the following parties: end users (including those responsible for procurement of the assembly or appointment of contractors); main contractors; site erection contractors; design consultants; control and instrumentation contractors; piping contractors; commissioning teams.


Quantock Trekking Holidays offers 2-day escorted riding holidays in the heart of the Quantock Hills. You'll stay in our purpose-built luxury accommodation Bashford Lodge, surrounded by stunning scenery and forests.
Take a riding holiday across the beautiful Quantock Hills, an Area of Outstanding Natural Beauty.
Our luxury new accommodation Bashford Lodge is the perfect sanctuary after a day of riding.
Get in contact and we'll tailor make a riding holiday to suit you and your group's abilities.
"I couldn't recommend a better place to spend the most relaxing weekend in 5* accommodation with excellent horses, amazing scenery, and wonderful people."
"Thank you both so much for the superb cooking, fantastic horses, and beautiful scenery!"
"I just wanted to say thank you, on behalf of all of us, for a fabulous weekend.
Everything was perfect - from the home cooked meal on arrival to the final mouthful of cake before we left!"
"Thanks again to you all for an amazing weekend. I was grinning all the way back to London, Dave's turbo-charged magical mystery tours will be very hard to beat! x"


Last week's episode of Nip/Tuck had an encounter between one of the plastic surgeons and an IRS auditor unlike any I have have ever seen or heard of. It's wacky enough to amuse taxpayers, tax pros, and IRS employees.
Click here if the embedded player doesn't work for you.


text:
Articles with section stubs, Monsters, Super Bomberman,
Bomberman World
Bomberman Tournament
Bomberman Portable
Bomberman DS
Super Bomberman Series
Mechabomb
Super: 800[1]
Super 2: 100, 200 (Red)
Super 3: 400
Super 5: 300[2]
Super Bomberman, Super Bomberman 2, Super Bomberman 3, Super Bomberman 5, Bomberman Quest, Bomberman World, Bomberman Tournament, Bomberman Portable, Super Bomberman R
Mechabomb is a somewhat common enemy in the Bomberman series. It is an exploding mecha that takes the form of a bomb with eyes. Notably, it is one of the few enemies that can actually harm other enemies and obstacles.
Super Bomberman
Bakuda (バクダ) moves slowly, turning or reversing direction upon colliding with a bomb or wall. Periodically, it will stop, turn into a normal bomb, and explode with a 3 Fire blast range before continuing its movement pattern.[3] It cannot be harmed when it is on the ground and ready to explode, but it can still be taken out when it is preparing to sit down. While on the ground, it takes about three to four seconds before it explodes.[4]
Bakuda Red (バクダレッド, Bakudareddo) is essentially the same as Bakuda, but its explosions will pierce through Soft Blocks and other obstacles. Although this makes it more dangerous than its regular counterpart, it is worth the same amount of points.[5]
Bakuda II (バクダII世, Bakuda II yo) moves slowly, randomly turning at corners. If the player comes within its line of sight and there are no obstacles between the two of them, it will move in the direction of the player. Periodically, it will stop, turn into a regular bomb, and sit down before exploding. It has a 4 Fire blast range. [6]
Bakuda Red II (バクダレッドII世, Bakudareddo II yo) is identical to Bakuda II, but its explosions pierce through Soft Blocks and other obstacles, and it has a 10 Fire blast range. It is worth twice as many points as its regular counterpart.[7]
Megadon (メガドン) moves at a normal pace, randomly turning at corners. It will often stick around the same area for extended periods of time. Like its previous incarnations, it explodes periodically, but its explosions is comparatively faster, with no moment of invulnerability. Its explosion has maximum range and will always extend to the nearest obstacles. They also explode when defeated. Notably, while they appear in normal stages, Megadons are also spawned by Professor Bagura in the final boss fight.[8]
In this game, the regular Bakuda from Super Bomberman appears in Zone 1. Its behavior is unchanged.
Mechabomb moves slowly, randomly turning or reversing at intersections. If it comes in line with the player and there are less than three tilespaces between the two of them with no obstacles in the way, it will stop, flicker, and then detonate. It is still vulnerable to attacks while it is preparing to explode. When it is defeated, it will explode. It has a 3 Fire blast range.
During the final boss battle, God-Header can turn regular bombs into Mechabombs. These Mechabombs quickly pursue the player and detonate when they get close, destroying themselves in the process. They pause and flicker shortly before detonate. They each have a Fire range of two. If they are hit by an explosion, they will stop moving and enter into their detonation mode, but they yield no score increases.
Mechabomb (メカメカドン, Mekamekadon) alternates between pursuing the player at a moderate pace and throwing bombs at the player. Because it moves directly toward the player, it will not move around walls, and thus can be "trapped" on the opposite side of a pillar or bomb. It has 5 HP and yields the Power Glove upon defeat. [9]
Mekadon (メカドン) hops quickly from tilespace to tilespace, weakly following the player. It explodes periodically,[10] and has a max blast range with explosions that pierce Soft Blocks and other obstacles. If Mekadon is hit by an explosion while it is sitting on the ground and preparing to explode, it will immediately explode, but it will not be harmed.
This section is a stub. You can help by expanding it.
Mechabomb moves slowly, randomly turning or reversing at intersections. At set intervals, it will stop, turn invulnerable, and ignite into an explosion. It does not explode upon defeat. Later stages replace it with a spiked, piercing variant, whose explosions act similarly to Bakuda Red of previous games. In this game, Mechabomb has been redesigned to be holding a torch.
The name "Bakuda" is derived from the Japanese word "bakudan", meaning "bomb".
"Don" is a Japanese sound effect that can be used for explosions.
↑ Super Bomberman Hudson Soft Guidebook, pg. 26
↑ Super Bomberman 5 Hudson Soft Guidebook, pg. 15
↑ Super Bomberman Complete Encyclopedia, pg. 90
↑ Super Bomberman 2 Hudson Soft Guidebook, pg. 27-28
↑ Bomberman Story Official Guidebook, pg. 77
Retrieved from "https://bomberman.fandom.com/wiki/Mechabomb?oldid=38209"
Articles with section stubs


text:
A.J. Fletcher Opera Theater Celebrates Grand Opening
A.J. Fletcher Opera Theater Celebrates Grand Opening Gala
The Fletcher Opera Theater opened to a capacity crowd. The A.J. Fletcher Opera Theater greeted its first audience on Thursday, February 22, with a performance by soprano Dawn Upshaw. Complete with a champagne reception the evening festively introduced the Triangle area to state-of-the-art acoustics and elegant construction in an intimate 600-seat setting. The capacity crowd was mesmerized by Upshaw's performance and the theater itself.
Barbara Goodmon (center) joined Dr &. Mrs. Assad Meymandi at the gala. The other wing of the new center bears his mother's name: Meymandi Concert Hall.
Floyd Fletcher (son of A.J. Fletcher), Margaret Fletcher (widow of A.J. Fletcher) & Jim Goodmon (grandson of A.J. Fletcher) settle into their box seats before the performance.
Former director of the National Opera Company Don Wilder helped celebrate the opening.
CBC's Whit Neville chats with the retired AJFF's Mary Beth Deaton before the show.
Jim Goodmon, son Jimmy & wife Barbara greet Dr. Meymandi on the front steps of the new Theater.
The A.J. Fletcher Opera Theater is part of the BTI Performing Arts Center. The Center also includes Memorial Auditorium & the new Meymandi Hall & Kennedy Theater.
A plethora of guests from Capitol Broadcasting and the A.J. Fletcher Foundation sat in box seats and celebrated the opening of the theater baring the name of the man who made WRAL a household name. Fletcher's mission of bringing the opera to the people of North Carolina took on new meaning with this grand opening celebration.
The icy night provided an elegant backdrop for the evening of opera.
AJFF's Waltye Rasulala eagerly awaits Upshaw's performance.
AJFF's Tom McGuire (right) contributed long hours to making the Theater a success.
CBC's Whit Neville & John Brennan visit with the guests at the champage reception.
CBC's Mike Hill & wife Melinda looked forward to attending the formal affair.
PrevPreviousOne Year Online For Nonprofitxpress
NextPelicans Food Services Community Horry County Children Continue To BenefitNext


text:
920 South 2nd Street,
2017-18 Student/Staff Calendar
District Special Programs
Volunteer Program (VISITS)
MVSD Equity & Nondiscrimination
The Mount Vernon School District is located 60 miles north of Seattle in the fertile Skagit Valley. We are a growing and diverse school district that employs nearly 900 people serving 6,200+ students in grades kindergarten-12. We have Six elementary schools (grades K-5), two middle schools (grades 6-8), one high school (grades 9-12), and one home school parent partnership (grades K-12).
Northwest Career
& Technical Academy
Harriet Rowley
Skagit Academy
SpEd Staff Portal
Childfind
Occupational / Physical Therapy Resources
Children with disabilities (birth to age 21) have a wide range of programs available based on their particular need. Special education services are delivered in regular classrooms, and in self-contained and resource room settings. Services are available at all schools including speech/language therapy, occupational and physical therapy, psychological assessment, and home-based instruction. Programs may be on a Mount Vernon School District site or at another educational location. Every student who receives special education must have an individual Education Program (IEP) developed by teachers, parents, and other professionals. For more information, contact Special Services at 360-428-6141.
Website feedback, questions, or concerns about accessibility
920 South 2nd Street, Mount Vernon, WA 98273 | Ph:360-428-6141 | Fx:360-336-2715


text:
The scene you see (left) could be the tailrace from a western water storage facility, but it is the tailrace fishery beginning at Buford dam below Lake Lanier just north of Atlanta.
The impact of this tailrace fishery and many like it across the southeast US is felt economically in many diverse ways. This article will focus on Southeastern stocked trout and the part that trout fishing actually plays in our economy. I believe that the facts in this article will surprise you.
I have heard that if you want to be in the fly fishing industry, and want to have a million dollars, just start with two million dollars and give it a year. You'll have one million dollars. There is, however, big money in fishing! The following article was written by Craig Springer of the U.S. Fish and Wildlife Service, southwest region. Craig has touched on a subject near and dear to all of us fishers in the southeastern USA -- the economics of trout fishing in the SE USA. - Bill Byrd.
You want to talk economic stimulus?
A Southeast study reveals some $107 million a year is spent directly on fishing, which generates another $212 million in related spending. That is $319 million of economic impact in the Southeast alone!
Brown and rainbow trout make it to creels of attentive anglers like those (right) throughout the Southeast, thanks in large part to federal hatcheries. If it were a corporation, it would be among the Fortune 500 companies, ahead of some heavy weights like Dow Chemical and Microsoft. More than 35 million Americans like to fish, and anglers spend money - lots of it. Money spent fishing sends concentric rings outward through the economy, spreading the wealth to businesses that often are only tangentially related. A recent economic study on the effects of trout fishing in the Southeast U.S. brings to light just how wide the rings ripple.
According to U.S. Fish and Wildlife Service economist Jim Caudill, expenditures by trout fishers in the Southeast have a tremendous effect on local and regional economies. More than $107 million a year is spent directly on fishing, rising directly from six national fish hatcheries that produce trout. That money, in turn, generates another $212 million a year in related spending. "It's not just the bait dealer, it's the gas station owner, it's the hotel proprietor and restaurant owner that feel the effects of fishing," said Caudill. "There's a multiplier effect in the economy from an activity that is enjoyed by a large number of people." Even the ladies are getting in on the action! Jodi Berlin (above left) is a guide and active fly fisher in Atlanta.
Fishing is big business and money spent creates more jobs. According to Caudill, 2,800 jobs in the Southeast - a direct result of fishing for brown, brook, rainbow and cutthroat trout - generate an annual payroll of $56 million. That's not just money in someone's pant pocket. This spending puts money into state and county treasuries: $6.8 million are collected each year in state sales and income taxes, and another $5.4 million goes to federal income taxes.
All of this economic activity, and the spending of money comes from what seems like an initial paltry investment of $2.1 million spent by the six national fish hatcheries to produce trout. Cold tailwaters are uniquely suited to support trout in the warm Southeast. "You can distill the effects even further," said Caudill. "For each dollar spent producing trout at these six national fish hatcheries, it generates through the economy upward of $140 in economic effects. Attendant to that is another $7.85 in tax revenue."
Trout fisheries in the Southeast are of recent vintage. Dams built by the U.S. Army Corps of Engineers and Tennessee Valley Authority essentially converted the warmwater bass and bream fisheries to cold water fisheries. The tailwaters below dams are cold given that the water releases come from the bottom of deep reservoirs. Trout, which favor cold water, were the natural replacement. Several of the U.S. Fish and Wildlife Service's national fish hatcheries were created to meet the demand for trout fishing. Erwin National Fish Hatchery in Tennessee is a brood stock hatchery. It, along with Ennis and Saratoga national fish hatcheries in Montana and Wyoming, send live trout eggs to Greers Ferry (AR), Norfolk (AR), Dale Hollow (TN), Chattahoochee (GA), and Wolf Creek (KY) national fish hatcheries, where the trout are grown out to catchable sizes and stocked over 10 southeastern states.
The western U.S. doesn't have a lock on trout fishing. More and more trout fishers are realizing that trout fishing has become a part of the sporting life in the Southeast for trout fishers like this one (right). What's good for the soul - recharging your batteries with a solo or family trip - is good for southeastern cash registers. Think of it as a mutual fund with a high return for the American people. The U.S. Fish and Wildlife Service operates 70 National Fish Hatcheries, along with 64 Fishery Resources Offices, nine Fish Health Centers, and seven Fish Technology Centers across the country.
Thanks to Craig Springer (LEFT) for this elightening article. Craig Springer is a fisheries biologist with the U.S. Fish and Wildlife Service in the Southwest Region.
He covers 17 field stations that work with anything from paddlefish in the Mississippi to rare Apache trout in the Arizona high country. Springer can be reached at his office (505 248-6867).
| LIGHT/ULTRALIGHT | WARM WATERS | RIVERS | SALTWATER |
| TECHNICAL | | HOME |


text:
Agitating Assam farmers reach Delhi to take part in protests
A section of farmers from Assam reached Delhi to take part in the 'Kisan Ganatantra Parade' that was planned today to march towards the national capital from Singhu border.
The march was organised to repeal the three contiguous farm laws introduced by the government of India in October last year.
The leader of the farmers' contingent from Assam while speaking said "We, the farmers of Assam, have just reached the protest in Delhi amidst a lot of challenges and we have brought pithas and other eatables for the langars here. We stand with our farmer brothers and sisters and have come today to repeal the farm laws."
The farmers from Assam were welcomed by Yogendra Yadav who has been supporting the farmers' protest since the beginning of their demands.


Keep your body healthy! It's your home where you have to live in.
Today, people are so busy running from one place to another, having stressful days, sitting for hours at the desk, grabbing something to eat on their way and ignoring the most important thing. Health! Take care of your body every single day.
You have this body to live in for the rest of your life so you better keep it healthy. If you are healthy you can do everything you want. Think of it this way…imagine your body as a crystal ball. Once it has a scratch, a crack or it's broken there's no way back!
An unhealthy body has limited actions. Sure, our body is an amazing thing and can heal itself. Like a small injury.
But, if you don't pay attention to that injury it may develop into a serious problem that your body won't be able to heal by itself. And even if it does you may remain with problems for the rest of your life.
This is one of my favorite quotes …and you know why? Because Van Damme is right. You have this body you live in and it's up to you to take care of it. And exercising it's a good way to do it.
Want to know how exercise can make you better, happier and healthier? Keep reading and you'll find out.
Treat your body with care, listen to it, don't neglect it. Even if it's just a minor pain. Untreated it may become worse…like when you're having a tooth ache. Don't wait until the pain becomes unbearable thinking it will go away. You'll end up losing your tooth.
Usually when something hurts, something in your body went wrong and the pain it's the way your body communicates with you. So pay attention to what your body is telling you.
Exercising is an amazing way to get your body healthy. Hard to believe but this can make you succeed in your every day challenges. You'll improve the quality of your life, your image, your whole body will benefit.
Working out not only shapes and designs your body making it look awesome…but also improves your mood your health and your attitude. It will improve your heart, your mobility, boost your immune system, give you more energy and it will make your whole life better. So how about some gym time?
I know it's not easy and there are excuses all the time. But if you don't make time for yourself today when will you? When it will be too late? There are so many types of sports and exercising and you are free to choose whatever makes you happy.
Too many people have a sedentary life. Sitting for hours at the office and at home it's not good for your health. I hope the reasons above will motivate you to lead an active life. There are so many benefits so why not enjoy them?
If you don't like going to the gym you can work out in the comfort of your home or outside…whatever suits you. Just make sure you have the proper equipment and you do the exercises the right way.
Excess body weight can put your health at risk. For example…it puts a lot of stress on your joints and heart. But you know this don't you? You hear it everywhere.
So you want to hit the gym? Keep in mind that just exercising without a proper diet won't get you results.
Lots of people see the word "diet" as something scary to do for a while. A good diet to me means healthy eating. And that's a way of life not just something for a few weeks.
Exercising combined with healthy eating will improve your immune system and your ability to move. It will keep your heart in shape, make bones, joints and muscles stronger.
Eating healthy and working out will also boost your mental health and keep diseases away.
In a word it will make you HEALTHIER.
Health is necessary for your body to function properly. To have a healthy body you need to have a healthy lifestyle and that may require some changes in your life so it's important to have your priorities straight. Put your health on the first place not other things because you won't be able to fully enjoy those things with a bad health.
Mental health is also very important and has a big impact on every aspect of your life including your physical health. We all know that stress can give stomach problems for example.
Work out and get that stress away! You'll sleep better, feel better, look better! A fit body will make you feel stronger and confident. Don't let stress ruin your life.
Today it's easy to get lost and forget to really live. Give yourself some free time. Learn to enjoy every day and make the best of it.
You can't really be happy and enjoy life if you're not healthy. We tend to forget about us, about our body, our health and why? You have the power to make things better!
Exercising, eating healthy and making the necessary changes for a better life won't be easy… it requires time, dedication and willpower. But the results will be awesome. So are you ready for a better and healthier you?
Keep your mind and body healthy. Eat properly, drink water, get enough sleep, exercise and let your body rest when it needs to. Remember prevention is better than cure !
Don't push it over the limit thinking it won't happen to you.
One more thing to keep in mind…make sure you ask your doctor before starting any form of exercising, especially if you know you have or had some health problems.
Thanks for the great reminders in taking care of our precious bodies. I have to admit that some days I do better than others!
I wonder why everything else is more important than our health? I admire people who seem to get the balance right.
Good question ! From my experience, I think people are not aware of the importance of a healthy body until they have a problem. Even if you are healthy you need to take care of your body to keep it that way.
Some don't even know how to take care of it. They don't know what it's good or bad or too much. When you're healthy, you don't worry about your body and you think it will never happen to you. Some people just don't care.
Thing is…many don't know this, especially when you're young. So an education on health is very important 🙂 What do you think?
I keep on telling this to all my colleagues. Unfortunately most of them believe life is meaningless if they cannot eat whatever their favourite items. Wish to forward this to some of them to who my advice sounds crazy.
Some people have the wrong idea about living life to the fullest. I totally agree with the idea to live and enjoy each day as much as you can, but destroying your health by making excesses isn't a good idea. One thing I learned is that you can't help someone who doesn't want to be helped.
Excellent post Cristina. The first step to a happy life is a healthy life. To me, health is the most important aspect of our lives. Without it, we can't enjoy any of what life has to offer us — money, love, friendship, success, etc. It's also one of the very few things that money cannot buy.
This is good stuff. sometimes we forget the simple things "taking care of your body".
Note to self: DO what Cristina said!!!
Great writing… a healthy mind and body are as important as long as we live on the earth.
Very important things in this post.. you need to listen to your body – thanks for posting!


There's going to be a live show on Thursday 17th February at Webstock the time and location haven't been confirmed, but anyone who can be there will know about it (as the location is being kindly provided by Webstock, only Webstock ticket holders will be able to get in).
Be there if you want to watch the train wreck as it happens, live on stage.
Discourse Guest: Robyn Gallagher, all about PACE, which she wrote about in a guest article on Public Address.
Do you know any Scientologists, former Scientologists, or cult busters? Tell them to get in touch. We'd like to do a special.
Next Next post: Episode 19: Live from Webstock!


text:
Home > Business > Jaro Education Fake – Not to Pay Attention to such News
Jaro Education Fake – Not to Pay Attention to such News
The growth of eLearning platforms has transformed the education sector. In India, the EdTech sector is evolving rapidly and is bridging the gap between talents and quality programs quite comprehensively. One of the leading companies in the business, Jaro Education is among the top 500 EdTech companies globally. It is renown for introducing a range of upskilling programs from diverse domains. It's a developing platform for learners around the world and the company is amplifying professionals with quality executive education.
For some time now, India's most trusted online higher education platform is facing challenges. Users are coming with doubts related to Jaro Education Fake. We hereby requested such readers to not follow such unauthorized links. All such content like Jaro Education Fake is fanciful news and you should not pay attention to such useless and fake information.
Why Should Students Not Trust Jaro Education Fake News
The renowned and reputed EdTech platform sticks only to ethical practices to achieve its business goals. It is among the fastest-growing EdTech companies in India. The firm also made an international impact by widening its academic collaborations with top global universities, B-schools and educational institutes.
They focuses on reshaping the growth of individuals by introducing programs. Hence, they focus to develop the skills of aspirants having desire to enter into fields. The fields like business management, data science, business finance, business analytics, banking & finance, IT sector, human resource management, FinTech etc.
How Jaro Education Successfully Gained Reputation in the Industry
Jaro Education is consistently coming up with outstanding programs to upgrade the skills of professionals. They guide them to build a career with globally recognized certifications. In today's world, when businesses are evolving rapidly, it is, therefore essential for individuals to possess in-demand and industry-relevant skills. They should adopt the much-needed training that helps them to grow as a professional. They develop a solution-oriented approach to find relevant solutions to typical modern-day business challenges. Hence, it's wise for aspirants to not look for unauthorized links like Jaro Education Fake. Always rely only on authentic information to get details about the company.
With the mission to continuously innovate in products, programs, and processes, Jaro Education builds the highest levels of operational efficiencies to maximize customer value. It holds the laurel of being the best by focusing only on innovations and value creation. With more than 12 years of industry expertise, the reputed EdTech player has a magnificent track record of more than 30,000 alumni. All these successful candidates have accomplished the mission of acquiring the most valued skills and now have developed the ability to find solutions to complicated and nuanced business problems. The programs offered by the company encourage students to glean pragmatic insights and develop leadership qualities to lead bigger teams. Instead of getting trap in rumours related to Jaro Education Fake, it's better to enquire more about such upskilling programs.
Jaro Education Earned a dignified image in the sector
In the era of digitalization, technology is undoubtedly an integral part of our lives. People find different ways to take advantage of it. It's good until it is used for a good purposes but today, people and organizations are using it for targeting their rivals. Jaro Education Fake is also a result of this business strategy. Rivals continue to weaponize information and develop increasingly sophisticated tools for personalizing, tampering and targeting any content in order to achieve business goals. This includes some forms of automated accounts used for astroturfing, networks of fake followers, targeted advertising and much more. All such form of false, inaccurate, or misleading information is leading to intentionally cause harm to a rival's reputation.
Though Jaro Education has earned a dignified image in the sector and its reputation is undoubtedly the best in the industry. People still get deflected with false content like Jaro Education Fake News. Our team has explored various aspects of such news over the web. It is seen that there's no reality behind any content related to this information. We have also conducted a ground check of this news and have collected the views of employees and Jaro Education's alumni. We compiled a list of views that frequently led us to the conclusion that this is a fascinated story made intentionally to tarnish the reputation of a leading EdTech platform.
Our readers are sensible enough to evaluate how a trusted company having such a magnificent track record and expertise of more than 12 years can indulge in such cheap practices. For Jaro, creating a superior technology and wide knowledge network is the only mission to enable an affordable, highly valued, and recognized world-class online program for professionals.
No matter how much effort middlemen put to spread the defamatory news about Jaro Education. The reputed firm Jaro Education has succeeded and gained a reputation in the industry.
Tags #Jaro Education #Jaro Education Fake #Jaro Education Fake News
Why the SMD screen is the best choice for Pakistani consumers in 2022
Best Methods To Improve Search Engine Rankings. Beginners Guide
What are the requirements for an udyam enlistment?
The Ultimate Guide To Buying Headphones And Jabra Headsets
Aerogel Market Analysis by Industry Size, Future Evolution, Scope and Analysis 2022-2027
The effect of working from home on the ownership of a house
Your Guide to a Successful Instagram Live Strategy in 2022
Data Center Switch Market Size 2022-2027, Share, Industry Trends, Opportunities, Analysis