text:
\section{Introduction}

The Josephson effect between two weakly coupled superconductors and the
steady flow of supercurrent in a perfect lead constitute the two main
paradigms of superconducting transport.
Both regimes can be viewed as the limits
of a general scenario in which Cooper pairs
flow coherently  in the presence of a scattering
obstacle of arbitrary strength.
The Josephson effect corresponds to the limit in
which a strongly reflecting obstacle
(typically, a tunneling barrier \cite{josephson} or a
point contact \cite{likharev})
reduces drastically the effective coupling between two
bulk superconductors while still preserving global coherence.
In the absence of an external bias, the current is given by the
Josephson relation
$I=I_C\sin(\Delta \varphi)$,
where $\Delta \varphi$ is the phase difference
between the two superconductors. The opposite limit is that of
supercurrent flow in
a perfect lead without appreciable scattering. In the appropiate gauge,
this regime is characterized
by a superconducting gap of uniform amplitude and
a linearly varying phase
whose gradient is proportional to the current. Specifically,
in the Ginzburg-Landau
limit, the current density can be written
$j=(e\hbar/m)|\psi|^2 \nabla
\varphi$, where $\psi=|\psi|e^{i\varphi}$ is the superconducting
order parameter.

An adequate measure of
the scattering strength is the average transmission
probability $T_0$ for a Fermi electron
passing through the barrier or contact in the normal phase,
\begin{equation}
T_0\equiv (h/e^2R_N)(2\pi/Ak_F^2)
\end{equation}
where $R_N$ is the device normal resistance, $A$ is the
cross section area of the
semiinfinite leads, and $k_F$ is the Fermi wave vector.
``Weak" and
``strong" superconductivities
are then characterized by $T_0 \ll 1$ and $T_0
\simeq 1$, respectively.
For a structure in which superconductivity is not weakened by
one-electron reflection, such as a {\it S-N-S} junction without current
concentration, a more general parameter is $I_C/I_B$,
where $I_C$ is the critical current of the structure and $I_B$
is the bulk critical current of the perfect lead.
It seems natural to ask
how is the superconducting flow for intermediate values
of $T_0$ or, more generally, $I_C/I_B$, i.e.,
how is the crossover between the two extreme
limits of superconducting
flow.
This rather fundamental question is of special current relevance, in
view of the recent activity on superconducting mesoscopic structures
(see, for instance, Refs. \cite{c1,c2,furu}).
In the case of a superconducting
point contact, the intermediate regime would correspond
to contact widths not much smaller
than the width of the semiinfinite leads. Alternatively,
in the case of tunneling
barriers, the crossover could be explored by considering
different degrees of transparency at the Fermi level. In the
case of a {\it S-N-S} junction, the intermediate behavior would be
displayed by relatively thin normal metal layers located between
two superconductors.

A preliminary version of some of the results contained
in this article
has been briefly presented in Ref. \cite{lt20}.

\section{Self-consistency and current conservation}

Theoretical studies of weak superconductivity
almost invariably assume that the phase is constant
within the two superconductors.
This is generally a reasonable approximation, since, by
definition, in this regime, $I_C \ll I_B$. As a
consequence, the variation of the phase in the bulk of the superconductor
displayed by current carrying solutions can be safely
neglected in a wide range of length scales.
It is clear that the approximation of
an asymptotically uniform phase cannot be justified
if $I_C$ becomes
comparable to $I_B$,
which will certainly be the case in structures with moderate
or negligibly weakened superconductivity.
The more general situation will be that of a phase
which varies linearly throughout the lead except
in a finite region near the scattering center where it varies
faster.

In order to discuss some general questions related to
self-consistency,
we focus in this section on structures in which the decoupling
between the two sides of a superconductor is due to
one-electron scattering by a barrier or point contact.
The conventional way of generalizing the BCS theory to the
presence of an arbitrary one-electron potential is based on the
Bogoliubov -- de Gennes (BdG) equations \cite{dG}:
\begin{eqnarray}
\left[ \begin{array}{cc}
H_0 & \Delta \\
\Delta^* & -H_0^* \end{array} \right] = \epsilon_n
\left[ \begin{array}{c} u_n \\ v_n \end{array} \right],
\end{eqnarray}
where $H_0$ is the one-electron Hamiltonian, $\Delta$
is the gap function, and $[u_n({\bf r}),v_n({\bf r)}]$ and
$\epsilon_n>0$ are, respectively,
the normalized wave function components and the energy of the
quasiparticle $n$. The self-consistency condition for
the gap function is \cite{dG}
\begin{equation}
\Delta = V \sum_{n} u_n v_n^* (1 - 2 f_n),
\end{equation}
where $V$ is the electron-phonon coupling constant and
$f_n=[\exp(\epsilon_n/kT)+1]^{-1}$.
The BdG Hamiltonian can alternatively be written
\begin{equation}
H = -\sum_{n\sigma}\epsilon_n \int \! d{\bf r} \, |v_n({\bf r})|^2
+\sum_{n\sigma}
\epsilon_n \gamma_{n\sigma}^{\dagger} \gamma_{n\sigma},
\end{equation}
where $\gamma_{n\sigma}^{\dagger}$ creates quasiparticle $n$
with spin $\sigma$.
In terms of the quasiparticle operators, the charge and current
density operators are written
\begin{eqnarray}
\rho=&&e\{\sum_{n\sigma}|v_n|^2+\sum_{nm\sigma}(u_n^*u_m-
v_n^*v_m)\gamma_{n\sigma}^{\dagger}\gamma_{m\sigma} \nonumber \\
&& + \sum_{nm\sigma}u_nv_m\sigma\gamma_{m\sigma}\gamma_{n,-\sigma}
+ \sum_{nm\sigma}u_n^*v_m^*\sigma\gamma_{n,-\sigma}^{\dagger}
\gamma_{m\sigma}^{\dagger}\} \\
{\bf j}=&&\frac{e\hbar}{2mi}\{-\sum_{n\sigma}v_n^*\mbox{{\bf D}}v_n
+\sum_{nm\sigma}
(u_n^*\mbox{{\bf D}}u_m+v_n^*\mbox{{\bf D}}v_m)\gamma_{n\sigma}^{\dagger}
\gamma_{m\sigma} \nonumber \\
&& +\sum_{nm\sigma}v_m\mbox{{\bf D}}u_n \sigma \gamma_{m\sigma}
\gamma_{n,-\sigma} - \sum_{nm\sigma} v_m^*\mbox{{\bf D}}u_n^* \sigma
\gamma_{n,-\sigma}^{\dagger}\gamma_{m\sigma}^{\dagger} \},
\end{eqnarray}
where $e=-|e|$,
$\sigma=\pm 1$,
and {\bf D} is defined as
$f\mbox{{\bf D}}g \equiv f (\nabla g)\!-\!(\nabla f)g$.
In Eqs. (5) and (6), the
contributions from the condensate and the quasiparticles have been clearly
separated. The quasiparticle contribution can in turn be divided into
a part which conserves the quasiparticle number and a part which
does not. The non-conserving components will not contribute
to the expectation values $<{\bf j}>$ and $<\rho>$ but will play an important
role in the quantum fluctuations of the electronic charge and
current densities.

If one attempts to solve the BdG equations (2) in a given
structure subject to
the boundary condition that the phase takes certain
constant values on each semiinfinite lead,
one generally finds from (6) a nonzero value of the total
current. This general feature can be illustrated by solving exactly a
specific and very important example, namely, that
of a strictly one-dimensional
superconductor (i.e., with only one propagating channel for the
Fermi electrons)
with a barrier of arbitrary transmission $T_0$
at the Fermi level. In this model, the phase is assumed to be
uniform on each side of the barrier. A non self-consistent resolution
of the BdG equations at zero temperature yields the current
\cite{c2,tesis,HKR}
\begin{equation}
I (\Delta \varphi) = \frac{e|\Delta|}{2\hbar} \frac{T_0 \sin(\Delta \varphi)}
{[1-T_0 \sin^2 (\Delta \varphi /2)]^{1/2}}
\end{equation}
where $\Delta \varphi$ is the difference between the phases on each side
of the barrier.
Fig. 1 shows the
current $I(\Delta \varphi)$
for several values of $T_0$.
As the strength of the barrier decreases, the current departs from the
ideal Josephson behavior and its maximum is displaced towards $\pi$.
In particular,
when $T_0$  equals  unity, the current is given by the formula
\cite{c1,tesis}
\begin{equation}
I (\Delta \varphi) = (e|\Delta|/\hbar) \sin(\Delta \varphi/2),
\end{equation}
with $-\pi<\Delta\varphi \le \pi$ and periodicity $2\pi$.
This result is clearly not self-consistent,
since a uniform phase should
be associated with a
vanishing equilibrium current,
at least in the asymptotic region. Actually, a more detailed calculation
reveals \cite{tesis} that the current (6) is localized exponentially
around the barrier
in a region of width
$\pi \xi_0/T_0 \sin(\Delta\varphi/2)$, where $\xi_0=\hbar v_F/\pi|\Delta|$
is the zero-temperature coherence length.
This peculiar feature can be traced back to the existence
of a localized, current-carrying quasiparticle at the interface
\cite{c1,tesis}.
Thus, one finds that the equilibrium
current is nonzero near the scattering center and zero in the
asymptotic region.
In the steady state, this situation clearly involves
a violation of charge conservation.
Below we show that the relation between self-consistency
and current conservation is in fact a general property of the BdG equations.

The time derivative of the charge density operator
can be computed
by applying (4) and (5) to the relation $\dot{\rho}=(1/i\hbar)[\rho,H]$.
The result is
\begin{eqnarray}
\dot{\rho}&=&\frac{e}{i\hbar}\sum_{nm\sigma}\{
(\epsilon_n-\epsilon_m)(v_n^*v_m-u_n^*u_m)\gamma_{n\sigma}^{\dagger}
\gamma_{m\sigma} \nonumber \\
&+&(\epsilon_n+\epsilon_m)\sigma[u_nv_m\gamma_{m\sigma}\gamma_{n,-\sigma}
+u^*_nv^*_m\gamma^{\dagger}_{n,-\sigma}\gamma^{\dagger}_{m\sigma}]\}
\end{eqnarray}
which obviously yields $<\dot{\rho}>=0$, as expected from a stationary
scattering description (we have used the properties
$<\gamma^{\dagger}_{n\sigma}\gamma_{n'\sigma'}>=f_n \delta_{nn'}
\delta_{\sigma\sigma'}$ and
$<\gamma_{n\sigma}\gamma_{n'\sigma'}>=0$).
Combining (6) and (9) we obtain for the continuity
equation \cite{lt20,tesis}

\begin{equation}
<{\bf \nabla \cdot j}> +<\frac{\partial\rho}{\partial t}>=
\frac{2e}{h}\sum_{n\sigma}
\mbox{Im}\{\Delta^*u_nv_n^*(1-2f_n)\}.
\end{equation}
By comparing this result with Eq. (3), it becomes
clear that charge conservation is only
guaranteed when the self-consistency condition is satisfied.
In the language of Ref. \cite{kadanoff}, the BCS-BdG theory is
a conserving approximation only for solutions that satisfy the
mean-field equations. It is interesting to note that the
the condensate and
quasiparticle contributions to the electric charge
are not conserved separately, but only
the sum of the two,
and if the description is fully self-consistent. The relation
between self-consistency and current conservation has also
been noticed by Furusaki and Tsukada \cite{furu2}, who have
derived an equation similar to (10) in which condensate and
quasiparticle contributions are however not clearly separated.
This seems to lead to a misinterpretation. Unlike suggested
in Ref. \cite{furu2}, preservation of current conservation is
not achieved in general by merely converting quasiparticle
current into condensate current \cite{furu2,btk}, but by
truly implementing global self-consistency. A good proof of this
assertion is that, within a non self-consistent scheme, the
source term in Eq. (10) is generally nonzero even at zero
temperature,
when no quasiparticles exist.

Before we proceed further a few additional remarks go in place. In one
dimension, Eq. (7) is
incorrect when $T_0$ is not much smaller than unity. In particular, Eq.
(8) is clearly wrong, since no bound quasiparticle should exist in
the absence of a barrier. Of course, the main inconsistency
lies in the very assumption of an existing phase difference, which
cannot be maintained without a scattering obstacle (an abrupt change
in the phase cannot survive the implementation of self-consistency).
It will be seen in the following
section that the appropiate generalization of the concept of
phase difference to structures with arbitrary transparency is the
phase offset, in terms of which
the transparent limit will be quite different from (8).
In studies of superconducting quantum point contacts,
equations which generalize (7) \cite{c2} and (8) \cite{c1,furu} to the presence
of many transverse modes can be found. In these cases, the lack of formal
self-consistency is justified. The localized nonzero current
corresponds to the current in the vicinity of the point contact and the
vanishing of the asymptotic current describes
the widening of the contact into
the reservoir. Therefore, Eqs. (7) and (8), as well as their multimode
generalizations \cite{c1,c2,furu}, are correct as long as
$I_C \ll I_B$. This is the case when the number of propagating modes
in the contact is much smaller than the number of modes in the wide leads.

\section{Study of the crossover}

 From the discussion in the previous section, it is clear
that, in order to achieve a unified view
of the crossover from weak
to strong superconductivity, one must deal with self-consistent,
current conserving
solutions of the BdG
equations in which a nonzero current is
associated with a linearly varying asymptotic phase,
and allow for arbitrary critical currents $I_C \le I_B$.
Unfortunately, the self-consistent resolution of the BdG equations
for arbitrary currents is in general a demanding numerical task.
By contrast, the formalism of Ginzburg-Landau (GL)
provides a relatively simple method to learn
about the global properties of those self-consistent solutions.
Therefore, our goal in this section is to
study the
solutions of the GL equation for a one-dimensional superconductor
in the presence of a delta potential of arbitrary strength.
Specifically, we wish to analyse
the stationary solutions of the free-energy functional
\begin{equation}
F=\int dx[|\nabla\psi|^2/\kappa^2-(1-V_0\delta(x))|\psi|^2
+|\psi|^4/2]
\end{equation}
where
$\kappa=\lambda/\xi$ ($\lambda(T)$ is the penetration depth and $\xi(T)$ is the
temperature-dependent coherence length) and
Abrikosov units are used. In these units, $\lambda(T)$ is the unit of length,
the order parameter $\psi$ is measured in units of $\psi_{\infty}$
(absolute value of the bulk order parameter at zero current), and $(\hbar/m)
(\psi_{\infty}^2/\xi(T)$ is the unit for current.
The complete
crossover between weak and strong superconductivity
will be explored by considering {\it all values
of the scattering strength $g\equiv\kappa V_0$}
ranging from $g$ very large (ideal Josephson
behavior) to $g=0$ (uniform superconductor).
In Eq. (11), $F$ must be understood as the freen energy per unit
area. This model should give a fairly adequate
picture of a quasi-one-dimensional superconductor
(of width $w \ll \lambda,\xi$)
in which a (narrower) point contact \cite{c2}
or a normal metal island has been inserted.
A clean point contact at low temperature
could not be described by (11), since, in the weak superconductivity
limit, this structure yields a current-phase relation of the type (8)
\cite{likharev,c1,kulik} instead of the usual $\sin(\Delta\varphi)$
behavior.
On the other hand, the model (11) is not appropiate for a quantitative
description of tunneling barriers because, in the limit of large
$g$, the repulsive potential $V_0\delta(x)$ yields hard-wall boundary
conditions, which do not correspond to a
GL description of the metal-insulator interface \cite{dG}.
A similar model, with the $\delta$ function replaced by a square barrier,
was studied by Jacobson \cite{jacobson}, who however focussed on the low
current limit. Volkov \cite{volkov} also used a delta function to describe
a {\it S-N-S} junction but only analysed the small current case.

If we
factorize $\psi(x)=R(x)e^{i\varphi(x)}$, the GL equations take the form
\begin{eqnarray}
&&\kappa^{-2} d^2R/dx^2
+[1-V_0\delta(x)](1-j^2/R^4)R
-R^3=0\nonumber\\
&&d\varphi/dx=\kappa j/R^2
\end{eqnarray}
where the current density $j$ is a conserved number ($I=jA$).
We are interested in solutions which satisfy the
boundary conditions
\begin{eqnarray}
&&dR(x)/dx = 0 \nonumber\\
&&\varphi(x) = qx \pm \Delta\varphi/2, \;\;\;\mbox{for}\; x
\rightarrow \pm \infty
\end{eqnarray}

Current
conservation requires the
product $R^2\varphi'=\kappa j$ to be constant, which can only be
achieved with a {\it nonzero} $q\equiv\kappa j/R^2_\infty$ in the
asymptotic solution. The general solutions for $R$ and $\varphi$
are of the form
\begin{eqnarray}
R^2(x)& = &a+b\tanh^2[\kappa u (x_0+|x|)]\nonumber \\
\varphi(x)& = &qx + \mbox{sgn}(x)\{\arctan[\beta\tanh(\kappa u(x_0
+|x|))] \nonumber\\&& - \arctan[\beta\tanh(\kappa u x_0)]\}.
\end{eqnarray}
In Eq. (9), $a(2-a)^2=8j^2$, with $0\leq a \leq 2/3$,
$b=1-3a/2$,
$u=\sqrt{b/2}$, $\beta=\sqrt{b/a}$, and
$x_0$ is obtained from the matching condition at the site of the
delta potential, which gives rise
to the cubic equation
\begin{equation}
\sqrt{2b}\beta y_0 (1-y_0^2)
-g(1+\beta^2 y_0^2) = 0,
\end{equation}
where $y_0\equiv\tanh(\kappa u x_0)$
and thus only the solutions satisfying
$0\leq y_0\leq 1$ are of interest. The solutions turn out to be uniquely
parametrized by the phase offset $\Delta \varphi$, whose general
expression is
\begin{equation}
\Delta\varphi=2[\arctan(\beta)-\arctan(\beta y_0)].
\end{equation}
The resulting curve $j(\Delta\varphi)$
is displayed in Fig. 2.
The inset shows the critical current as a function of $g$.
The Josephson limit is well achieved for $g>8$ while $j_C$
saturates to $j_B=2/3\sqrt{3}=0.385$ as
$g\rightarrow 0$.
For large $g$, one finds the ideal Josephson
behavior, $j=j_C\sin(\Delta\varphi)$, with $j_C=1/2g$ taking small
values. For $g=0$, two types of solutions are obtained. One of them
is entirely expected: for $\Delta\varphi=0$, all currents are possible
ranging from $j=0$ to $j=j_B$. These are
the solutions of the uniform superconductor in which $\varphi'$ and
$R$ take constant values. The second type of solutions
are {\it the solitons of the $\psi^4$
theory defined by} (11)
{\it for arbitrary values of the current $j$} \cite{lt20}.
These kinks
separate two domains in which the phase varies linearly,
\begin{equation}
\varphi(x)=qx + \arctan[\beta\tanh(\kappa u x)]
\end{equation}
with a total phase offset of $\Delta\varphi=2\arctan(\beta)$.
It is interesting to note that, unlike in the $j=0$ case, the phase
offset (which here plays the role of the soliton charge) can
be different from $\pi$.
These solitonic solutions
are equivalent to the saddle-point configurations
which were considered by Langer and Ambegaokar \cite{la}
in their study of the resistive behavior of one-dimensional
superconductors.

Fig. 3 shows the behavior of $R(x)$ and $\varphi(x)$ for $g = 0.2$
and two different values of the current. In Fig. 3a, it is clearly
seen that, for
$j=0.01$, the solitonic solution almost vanishes at $x=0$. For the same
solution,
Fig. 3b shows that the spatial variation of $\varphi(x)$ is almost negligible
except for a step-like feature at $x=0$ (the phase can be shown to vary
in a length scale $j/\kappa$ if $j$ is small).
For $j = 0.35$ (close to $j_B$),
the phase displays a linear increase with $x$ with an offset due to a
faster variation in the vicinity of $x=0$.

An interesting feature of the $j(\Delta\varphi)$
curves which can be clearly observed in Fig. 2 is that,
as the scattering is turned off,
the maximum current is displaced towards lower values of $\Delta\varphi$.
This is in sharp contrast with the behavior shown in Fig. 1 for
the non self-consistent solutions. It has already been noticed that a
superconducting point
contact displays the same behavior as
its propagating channels evolve from low to high transmission
\cite{c2}.
There is of course no contradiction between our results and those obtained
for point contacts,
since the latter apply only in the limit $I_C \ll I_B$, while the low $g$
curves
in Fig. 2 are only relevant in the $I_C \sim I_B$ case.

Baratoff {\it et al.} \cite{bbs} considered a {\it S-}$S'${\it -S} structure in
which $S$ and $S'$ are two dirty superconductors of differing properties.
As a function of the similarity between $S$ and $S'$, they obtained
results which qualitatively resemble those obtained by us. However,
their focus was not in the crossover from weak to strong superconductivity,
but rather in the qualitative modeling of weak links. In particular, they
did not consider the $S=S'$ case and, although the relation
to Ref. \cite{la} is noticed, no association
is made between the branch to the left of the
maximum in the $j\!-\!\Delta\varphi$ curve and
the trivial solutions of the uniform case.
More recently, Kupriyanov \cite{kupri} has studied the
properties of an {\it S-I-S} structure
by means of the Usadel equations, which apply in the dirty limit.
He considers several
values of the barrier transparency and obtains results
which, after a nontrivial
scale transformation (the phase change across the barrier
instead of the phase offset is used as a parameter),
can be shown to be qualitatively similar to
those displayed in Fig. (2). However, in the transparent limit,
no mention is made in Ref. \cite{kupri} of the
relation to the solitonic solutions of Ref. \cite{la}
nor to the uniform solutions, as discussed here by us.

\section{Crossover in long bridges.  Breakdown of the ac Josephson effect.}

So far we have focussed on the relation between the current $j$ and the
phase offset $\Delta\varphi$, which uniquely parametrizes the solutions
of the GL equations (12). However, it is
also convenient to plot the current as a function of the total
phase difference $\chi$ between two reference points.
These two points can be, for instance, the
extremes of a superconductor of length $L$ with an effective barrier
in its center.
A typical case would be that of a narrow bridge connecting two
wide reservoirs through smooth contacts beyond which the phase gradient
can be safely neglected \cite{likharev}. For a given length
$L$, one can compute $\chi$ from the relation $\chi=\varphi(L/2)-
\varphi(-L/2)$. If
$L \gg (\kappa u)^{-1}$,
we can  approximate
\begin{equation}
\chi\simeq qL+\Delta\varphi.
\end{equation}
Since $u\rightarrow 0$ as $j \rightarrow j_C$,
there is a threshold current $j_{th}(L)$ above which
Eq. (18) does not apply.
For $\kappa L \gg 1$, $j_{th}\simeq
j_B(1-27/16\kappa^2L^2)$.
In Fig. 4, the resulting curve $j(\chi)$ is plotted for
$\kappa L=10$.
In such a case $(j_B-j_{th})/j_B \simeq 0.016$.
It can be observed that, for large $g$, the ideal Josephson
behavior is displayed, while, for sufficiently small $g$,
the current becomes a multivalued function of the total phase
$\chi$. The pattern shown in Fig. 4 is actually repeated
periodically with a period of $2\pi$. In the case of $g$ small
it becomes clear from the comparison with Fig. 2 that the
upper branch corresponds to solutions with a linearly
varying
phase ($\Delta\varphi\simeq0$), while the lower branch is
given by the solitonic solutions with a nonzero phase offset.
This feature has also been noticed recently by
Martin-Rodero {\it et al.} \cite{amr}, who have computed
numerically the self-consistent solutions of the BdG equations for
a linear chain coupled to two Bethe lattices at zero temperature.
The discontinuity in the derivative at the top of the $g=0$
curve in Fig. 4 reflects the discontinuous transition from
the uniform to the solitonic branch shown in Fig. 2.
However, this cusp cannot be observed in bridges of finite length since
it always lies above the threshold of validity of Eq. (18).

In Fig. 5 we display
the phase of
the order parameter as a function of the position and the
phase offset for $g=10$ (Josephson limit).
When $\Delta\varphi=\pm\pi$,
the current is zero. This requires an
abrupt jump of $\pm\pi$ at
$x=0$, which is possible because $R(0)=0$ in these
solutions, as can be proven quite
generally.
These are
the phase-slip configurations which permit the existence of the
ac Josephson effect.
As an external driving voltage is applied
between two points on different sides of the junction,
the phase  is forced to vary at a constant rate
and the whole sytem responds
adiabatically by evolving along the continuous set of stationary
solutions.
The existence of these step function solutions
makes it topologically possible for the phase at every
point to increase both monotonically and continuously
with time.
Since $R(0)=0$, the two superconductors are completely
decoupled and $\Delta\varphi=\pi$ is equivalent to
$\Delta\varphi=-\pi$.
As the system is driven by the external
bias through the different values of $\Delta\varphi$ and
reaches the value $\Delta\varphi=\pi$, it automatically
reenters through the topologically equivalent configuration
with $\Delta\varphi=-\pi$ and the phase at the boundary
can continue to increase monotonically. Thus the existence
of the ac Josephson effect relies on the ability of
the system to undergo adiabatic phase-slips under the action
of an external bias. It is interesting to note that, at the
particular value $\Delta\varphi = \pm \pi$, the configuration
of the order parameter is independent of
$g$, since then $R(0)=0$. In particular, it is identical to the
phase-slip configuration in the absence of a barrier, as studied
by other authors (see, for example, Refs. \cite{rieger,kramer}).

At zero current, all points on one
side of the
barrier have the same phase. In particular,
$\varphi(x>0)=\pm\pi/2$ for $\Delta\varphi=\pm\pi$.
By contrast, the solutions with nonzero current have an asymptotic
phase which grows linearly with position, as shown in Eq. (17).
Thus, for sufficiently large $x$, it is not possible to have
$\varphi(x)$ increasing monotonically as $\Delta\varphi$ varies between
the two equivalent configurations with $\Delta\varphi=\pm\pi$. As
a consequence, the system cannot respond
adiabatically
to a constant voltage being applied at points that are
sufficiently distant from the junction. The only choice for
the system will be to undergo nonadiabatic, fluctuating processes
of the type studied by Langer and Ambegaokar \cite{la} (albeit
with $g\neq0$), which will originate a resistive behavior.
The threshold for this type of response is given by the condition
\begin{equation}
\left.\frac{\partial\varphi(x_b)}{\partial\Delta\varphi}
\right
|_{\Delta\varphi=\pi}=0
\; \; \; \mbox{at}  \; \; \Delta\varphi=\pi
\end{equation}
If one identifies $x_b=L/2$ and $\varphi(x_b)=\chi/2$, this is also
the condition for
the onset of bivaluedness
in the $j(\chi)$ curve of Fig. 4, which requires
$\partial\chi/\partial j=0$ at $\chi=\pi$ (note that,
$\partial j/\partial \Delta\varphi\neq 0$ at
$\Delta\varphi=\pi$). Thus, if the electrodes are applied at
points $|x|>x_b$,
there is a breakdown of the ac Josephson effect
due to the fundamental inability of the system to respond
adiabatically to that particular type of external constraint.

Let us estimate the breakdown length $x_b$.
For $g$ large, one can show that $x_b\simeq g/\kappa$.
We notice at this point that the value of the parameter
$g$ can be adjusted to a realistic setup by exploiting the
relation
\begin{equation}
g=1.30\cdot(j_B/j_C),
\end{equation}
which applies
in the Josephson regime, and noting that $j_B/j_C=I_B/I_C$.
We have considered explicitly four types of structures which are
known to display a standard $\sin(\Delta\varphi)$ behavior
in the
Josephson limit
for $T$ close to $T_c$: (a) a tunnel junction with average
transmission $T_0$ for the Fermi electrons, (b) a clean point
contact with average transmission $T_0$, (c) a narrow bridge
between two superconductors
made of a dirty normal metal of length $L$ and coherence
length $\xi_N$ at $T\simeq T_c$, and (d) a {\it S-N-S} structure
without current concentration ($N$ and $S$ have the same width).
Cases (a) and (b) fall within the same category in the GL
limit, with an expression $I_C=\pi \Delta^2(T)/4eR_Nk_BT$ for the
critical current \cite{likharev}.
Noting that, for $T$ close to $T_c$, the gap
function and the order parameter are related by \cite{abrikosov}
$\psi=0.326\,\sqrt{n}\Delta/k_BT_c$, where $n$ is the electron
number density, we arrive at
\begin{equation}
g^{-1}\simeq 2.0 \; T_0 (\xi(T)/\xi_0).
\end{equation}
For case (c), the critical current is \cite{likharev}
$I_C=(4\Delta^2(T)/\pi eR_Nk_BT)(L/\xi_N)\exp(-L/\xi_N)$, if
$L \gg \xi_N$. Thus one obtains
\begin{equation}
g^{-1}\simeq 3.23 \;T_0 (\xi(T)/\xi_0)(L/\xi_N)\exp(-L/\xi_N).
\end{equation}
For a {\it S-N-S} structure without current concentration, the critical
current is \cite{abrikosov1} $I_C=A(e\hbar n/2m)(|T-T_c|/T_c)
(\xi_N/\xi^2(T))\exp(-L/\xi_N)$. As a consequence,
\begin{equation}
g^{-1}\simeq 10.6 \;(\xi_N/\xi(T))\exp(-L/\xi_N).
\end{equation}
Shifting to real units, we arrive at the relations
\begin{eqnarray}
x_b & \simeq & 0.50 \; \xi_0/T_0
\mbox{\hspace{3cm}(a),(b)} \nonumber \\
x_b & \simeq & 0.31 \; (\xi_0\xi_N/T_0L)e^{L/\xi_N}
\mbox{\hspace{1cm}(c)}
\nonumber \\
x_b & \simeq & 0.094 \; (\xi^2(T)/\xi_N)e^{L/\xi_N}
\mbox{\hspace{0.8cm}(d)}
\end{eqnarray}
for the maximum distance at which a constant voltage can be applied
in order to observe the ac Josephson effect.

\section{Conclusions}

We have studied the nature of
the crossover from ideal Josephson behavior between two weakly
coupled superconductors to bulk
superconducting flow in a perfect superconducting lead.
We have argued that a
self-consistent resolution of the BdG equations
is mandatory in a microscopic study of the crossover and have
proved that charge conservation is only guaranteed when
the requirement of self-consistency is satisfied.
We have performed a study of the crossover by
solving exactly
the Ginzburg-Landau equation for a
one-dimensional superconductor in the presence of a delta potential
of arbitrary strength. The pairs of Josephson solutions with equal
current have their scattering free counterparts in the pairs
formed by a uniform
and a solitonic solution. This relation has allowed us to understand
some aspects
of the  multivalued current-phase relation in
narrow bridges.
The complete knowledge of the set of stationary solutions for
different values of the scattering strength $g$ has helped us to gain
a more detailed understanding of the
adiabatic response to a constant external
bias, which has been shown to rely
on the feasibility of
adiabatic phase-slips.
If a voltage is applied at points which are sufficiently
far from the junction, there is a breakdown of the Josephson
effect due to the intrinsic impossibility of changing adiabatically
the phase
at a distant point in a continuous and monotonic manner.

\acknowledgments
The authors would like to thank P. Ao, C.W.J. Beenakker,
F. Flores, P. Goldbart, F.
Guinea, A. J. Leggett, A. Levi Yeyati, and A. Martin-Rodero for
useful discussions at various stages of this work. This project
has been supported by CICyT, Project no. MAT91-0905.

redpajama_set_name: RedPajamaArXiv


text:
ACCEPTED

#### According to
The Catalogue of Life, 3rd January 2011

#### Published in
Tabl. regn. veg. 3:547. 1799

#### Original name
null

### Remarks
null

redpajama_set_name: RedPajamaGithub


text:
Quantitative ultrasound measurements of bone speed of sound in premature infants
Eur J Pediatr. 2001 Dec;160(12):736-40. doi: 10.1007/s004310100849.
D Nemet 1 , T Dolfin, B Wolach, A Eliakim
1 Department of Paediatrics, Meir General Hospital, Kfar-Saba, The Sackler School of Medicine, Tel Aviv University, Israel.
DOI: 10.1007/s004310100849
We measured bone speed of sound in premature infants by quantitative ultrasound. A total of 44 neonates participated in the study including 29 premature infants (median birth weight 1264 g, range 578-2420 g; median gestational age 31 weeks, range 24-36 weeks) and 15 full-term infants (median birth weight 3360 g, range 2700-3730 g; median gestational age 40 weeks, range 37-41 weeks). The left tibial speed of sound (SOS) was measured by quantitative ultrasound. Bone SOS was successfully measured in all infants. We found a significant correlation between tibial SOS and gestational age (r = 0.78, P < 0.0005), but a significant inverse correlation between tibial SOS and post-natal age (r = -0.78, P < 0.0005). Bone SOS was significantly (P < 0.05) higher in full-term infants (3101 m/s, range 2899-3314 m/s) compared to premature infants (2821 m/s, range 2516-3139 m/s), and compared to a subgroup of the premature infants who reached corrected age of full-term infants (2706 m/s, range 2516-2892 m/s, n = 13). Bone SOS was lower (2745 m/s, range 2533-3036 m/s, n = 16) in very low birth weight premature infants (birth weight < 1500 g).
Conclusion: The results indicate that tibial speed of sound was reduced in premature infants (in particular very low birth weight) compared to full-term infants even when premature infants reached the corrected age of their full-term peers. The potential role of this technique in assessing osteopenia in premature infants warrants further exploration.
Alkaline Phosphatase / blood
Bone Diseases, Metabolic / blood
Bone Diseases, Metabolic / diagnosis*
Bone Diseases, Metabolic / diagnostic imaging*
Infant, Premature*
Tibia / diagnostic imaging*

redpajama_set_name: RedPajamaCommonCrawl


CHECOTAH, Oklahoma - Checotah native Carrie Underwood donated a great gift to her old high school on Saturday.
Underwood provided new stage curtains for the Checotah High Event Center which school officials say will be ready for everyone to see during their Meet the Teacher night on Tuesday.
"They look amazing and will give our students the great opportunity to experience a professional stage setting. Thank you, Carrie for supporting Checotah Schools and continuing to help make your hometown one of the best little towns in Oklahoma," said a Checotah official.


Have fun experimenting with your look when you wear this off-white shirt by Mufti. Its timeless appeal is accentuated by the slightly shaped hem, colourful tropical print and spread collar. A pair of dark blue jeans with this will complete your casual look.


Freight forwarders in Australia are the foundation of our business and the area in which we excel. International freight forwarding companies helps in importing and exporting, transportation by road, sea or air (or a combination of these three) and customs clearance. We offer a full range of services that will ensure your goods arrive at their destination – anywhere in the world – with steadfast care and as quickly as is humanly possible.
Here at TSL we are fully versed in the specialised and complex operation that is international freight forwarding. Freight companies in Melbourne have spent many years developing systems that cut out the complications, creating a highly effective and efficient service that's ready for you to make the most of. We are excited to work with you in order to improve your business.
Freight forwarding is a procedure that involves a number of different agents: the buyer, the vendor, the packer, the carrier, the transporter and customs. Because these services are so closely interlinked, there is a lot that can go wrong. Thanks to years of honing our systems and developing the very best professional links with all the entities along the freight forwarding chain, we have created a continuous process whereby everyone is working towards one thing: an effective, efficient operation. We are happy to share our experience with you and help you carry out your imports and exports in the most proficient way imaginable.
Choosing the right freight and logistics companies in Melbourne is essential for your business. Without a service provider whom you can put your trust in, you are putting your company and your reputation at risk. For this reason, we work hard to provide a service that helps you achieve your business goals and keeps your valued customers happy.
For further information, contact the friendly team at TSL Australia today, leading Melbourne freight forwarders. We look forward to working with you.
When you use our International Forwarding Services.


text:
Home Our Team Our Companies Investors
Home About Us Our Companies Investors
RDE, Inc.
(OTC: RSTN)
All Things Restaurant - Restaurants, Dining, and E-commerce
We guide our customers to easy savings within a few clicks—or taps!—on our sites. A variety of choices for customers is the way to building the future of participatory e-commerce!
WE VALUE OUR PARTNERS
We diligently maintain an extensive network of long-term partner relationships and we continue to prove our strategic methods add value to their businesses that they can't find elsewhere.
WE PRIORITIZE OUR CUSTOMERS
When our customers are hungry for savings, they come to us for the latest deals and promotions and that says a lot about our commitment to our mission.
Kevin Harrington - Board Member
Nearly 40 years experience in product introduction and direct marketing, being one of the first to market products through infomercials in 1984. A serial entrepreneur, Mr. Harrington appeared as one of the original panelists on "Shark Tank," from 2009 to 2011. He currently serves as a director of Celsius Corp., Emergent Health Corp., and Redwood Scientific Technologies, Inc.
5880 Live Oak Parkway Suite 100
© 2020 RDE, Inc. · All rights reserved.


text:
Q: add jointable "catalog_product_entity" It get error Can't retrieve entity config I modified a module ordergrid to add a column, "provider", that load a attribute from product. I added jointable('catalog_product_entity_int') to the code and I got a
Can't retrieve entity config: sales/catalog_product_entity_int
I have read about the same problem but these cases happens with new tables or blocks. I checked config.xml of another module that uses attributes from products and it does not declare anything about catalog_product_entity.
I assume is a declaration of xml problem but I did some changes and did not get anything.
Some idea??
Thanks.

redpajama_set_name: RedPajamaStackExchange


Professional international shipping of your household goods worldwide.
Your search for the Best Pennsylvania International Movers ends here.
We provide the best Pennsylvania International Moving & International Shipping Services.
Sea & Air Pennsylvania international moving company (888) 453 0941.
Philadelphia PA International Movers Get a Free Quotes Online Today.
We believe each international move is different and has its own specific requirements.
We are sensitive to, and look for those special requirements to be sure that your needs are fully understood and that we are prepared to provide the services required to assure your international move is seamless.
You will be assigned a Sea & Air representative to oversee your move, who will keep you informed every step of the way.
As a notable international mover, Sea & Air International has the benefit of decades of experience in international moving and shipping.
Thank you for considering Sea & Air International. for your upcoming relocation.
Providing clarity of our international mover costing which means you know there are no hidden charges.
Communicating the most accurate and timely advice before, during and after your international move.
Responding to clients' needs by assigning a dedicated, experienced international mover representative.
Delivering higher standards as an international mover across all points of contact for our clients.
Offering the most experienced packing crews who use the correct packing techniques and materials.
Meeting our clients' rapidly changing requirements by continuously investing in new technologies.
Maintaining an in-depth international mover training program for new associates.


AIG was running a scam that enabled companies to dodge paying taxes. Yes, the same AIG that is now sucking up our tax dollars – and paying out million-dollar-bonuses – was in the business of helping companies not pay their taxes.
At what point do we feel completely harvested, bled, scammed, and done with this? Why aren't we raising taxes on high incomes — the beneficiaries of all these scams that brought down the economy — to pay for all of this?
An attorney and tax shelter expert we spoke with today says AIG FP was one of the biggest players in the business of engineering offshore tax shelters for corporate and private clients that resembled a multibillion dollar tax evasion scheme called Son of Boss (we don't have time to figure out why) that thousands of corporations and wealthy individuals used to book phony capital gains losses and evade most or all of their income taxes in the late nineties and early 00s.
New court papers indicate that the American International Group helped dozens of wealthy individuals make use of questionable tax shelters intended to shield hundreds of millions of dollars in profits from federal taxes.
A.I.G. is under scrutiny by federal and New York investigators looking into questionable insurance transactions that the company used to dress up its financial strength.
How much of this economic mess is because We, the People didn't demand that this company be broken up when this news came out?
Why haven't We, the People taken control and broken these "companies" up into little bite-sized chunks yet?


text:
The Opus Group® Announces First Tenant at River Ridge Commerce Center Industrial Development
The Opus Group (Opus) announced today Denso Products and Services Americas, Inc. (Denso), one of the largest automotive parts manufacturers in the world, has signed a lease for Opus' completed industrial building in River Ridge Commerce Center in Jeffersonville, Indiana. Denso will occupy 311,483 square feet of the 426,450-square-foot industrial building.
"We were thrilled to work with Denso and provide them with a distribution solution that allows them to better serve their clients," said Douglas J. Swain, vice president, general manager, at Opus. "This is our first project in the greater Louisville market, and we look forward to bringing more industrial developments to this high-demand market."
The industrial warehouse at River Ridge Commerce Center is Denso's first facility in the greater Louisville market. The company chose the site so it can continue expanding operations in the future and gain better access to major transportation routes. The site will serve as a distribution center of Denso automotive technology systems and components to regional automotive manufacturers.
Located off State Route 62 with easy access to major freeways, Opus' building at River Ridge Commerce Center answers the rapidly growing demand for commerce and distribution warehouse space in the urban area. The building is located near the UPS Worldport Air Hub and features 32-foot clear height as well as 44 dock positions. The development also offers more than 300 car parking spaces and 49 excess trailer parking spots. An additional 114,967 square feet of space remains available for lease.
Opus was the developer, design-builder, architect and structural engineer of record on the project. Kevin Groves of CBRE represented Opus in the lease transaction.
About The Opus Group
The Opus Group® is a family of commercial real estate development, construction and design companies headquartered in Minneapolis with offices and projects across the country. Opus operates as an integrated, multidisciplinary team with expertise in development, capital markets and finance; project management and construction; architecture, engineering and interior design. The Opus Group includes Opus Holding, L.L.C. and its operating subsidiaries: Opus Development Company, L.L.C., Opus Design Build, L.L.C. and Opus AE Group, L.L.C. Specializing in industrial, office, residential, retail and institutional projects, The Opus Group has broad capabilities, deep experience and a proven design-build model that delivers solutions for customers on time and on budget. For more information, visit www.opus-group.com and follow @TheOpusGroup on Twitter and @theopusgroup on Instagram.
Filed Under: Indianapolis, Industrial Development & Construction, Spec Development


… is when you have to because you can't stand not starting it. It's been on your mind, you're sure it will work.
… was actually years ago; but the second best time is now.
… is when you've thought it through, you know the risks, and you have a good realistic sense of challenges, keys to success, and likelihood of failure.
… is when you're comfortable with your estimates of starting costs, sales, costs, and expenses. They feel like they are reasonable educated guesses.
… is when your spouse or significant other says "do it" and not "don't do it." Businesses fail and it's not always something you did or didn't do. Will failing at your own business kill important relationships?
… is when you gather up the money your business plan says you need to be able to start.
Don't worry too much about the larger economic, employment, and socio-economic trends. Your business depends on what you do. It's micro economics, not macro economics. Huge enterprises swing with the national economy, but small businesses depend on the specifics of what you do, how well you execute, and how well you communicate and deliver value to your customers.


This Holiday Romance white tea blend is a full blown Rio street carnival of succulent, mouthwatering infusions of sweet, juicy fruits. The robust, powerful flavours of the green tea are able to magically lift and enhance the more delicate aspects of the white tea without overpowering it. This gives a satisfying, rounded aroma of deep, vegetal scents at the core, enveloped in a tropical bouquet of enticing floral perfume and spirited, fresh nectars. Take a moment to prepare yourself for this experience - a rich medley of goji berries, cranberries and pomegranates, all of which have been infused to create the irresistible extravagance of this deep, red elixir.
Ingredients: White tea, Green tea, Flavourings, Papaya bits (papaya, sugar), Pineapple bits (pineapple, sugar, acidifier: citric acid), Goji berries, Cranberry bits, Kiwi bits.
Holiday Romance (Pomegranate Cranberry White Tea) 117.


The food and beverage industry in India is in a state of evolution as Indians are beginning to lay substantial emphasis on the nutritional value of edible products along with their taste. Fruits are best had when they are ripe for picking (as nature intended it to be), straight from the tree - at their nutritious and tasteful best.
In fact there is rising consciousness in the Indian consumer about the importance of a healthy lifestyle and the critical role that a healthy diet plays in it. As per market research commissioned by us, there are concerns among consumers about the prevalent unhealthy lifestyles, the nutritional value of the diet they are consuming, and their exercise levels being insufficient. Also, there are worries about the products that are being consumed, whether they have too many artificial ingredients or what role do the ingredients play in terms of adding nutrient value. Also, there has been a noticeable increase in the understanding of nutritional vocabulary and customers are no longer just accept blindly everything that is said to them.


Megan and I were extraordinarily blessed to speak with Robert Scheinfeld for this episode of Soulfullpreneur Radio. His books have made a huge impact on our lives and helped us to "Bust Loose" from conventional thinking and being. And it turns out…that was just the middle of the story!
Robert has a very interesting past and many gifts to share with the world.
For more than 20 years, Robert Scheinfeld has been helping people worldwide create extraordinary results, in less time, with less effort, and much more fun.
Robert captivates audiences through his unique and memorable personal stories of transformation and by sharing valuable and empowering insights from his own rich life.
Robert began his path to discovering True Success at age 12 when his tycoon grandfather (founder of Manpower, Inc. – the world's largest temporary help service and Fortune 150 company) told him True Success is based on your ability to tap power in "the invisible world." Unfortunately, his grandfather died before he could finish teaching Robert about the invisible world and other secrets of his success.
Scheinfeld, however, was determined to unlock the mystery of success by discovering the inner workings of his grandfather's invisible world. During his journey, Robert spent over 33 years on what he now calls "The Treasure Hunt of the Century." Along the way, he became a multimillionaire (and self-proclaimed stressed-out maniac), plunged $153,000 in debt, and spent seven years struggling before he solved the mystery his grandfather left him with at such a young age. His "Busting Loose" body of work reveals his discoveries and how you can apply them to create True Success in your life.
Along his journey, Robert became a master of applying cutting edge sales and marketing strategies and has had in-the-trenches experience of creating profitable million dollar businesses (on and off the Internet).
For example, Robert helped grow Blue Ocean Software from $1 million to $44 million in less than four years, resulting in the company being named three times to the Inc. Magazine Inc. 500 list. That tremendous growth, accompanied by outrageous profitability, led to Blue Ocean being acquired by software giant Intuit for $177 million.
He also played a key role in growing a computer store franchise company called Connecting Point of America from $90 million to $350 million in sales. In addition, the marketing model and system Robert created was used to pack the room at Tony Robbins multi-media seminars.
More than providing more of the "same old, same old" or another rah-rah motivational pump up job that doesn't last, an interaction with Robert empowers you to see with unusual clarity, act with newfound confidence, and transform the results you produce in your life and work.
He gets you on-track, laser-focused, and tapping into a new kind of power to finally experience the True Financial Freedom you've been searching for.
And at his thoughtfully constructed website, www.robertscheinfeld.com, you will find many more free resources and a few which require an expression of appreciation (moolah).
We hope that you enjoy this podcast as well as the extras that Robert is offering.


text:
Thursday's NCAA tournament rematch between UMass men's soccer and Colgate will be a battle of adjustments
By Amin Touri
(Jessica Picard/Daily Collegian)
The Massachusetts men's soccer team will play an NCAA tournament game on Thursday for the first time since 2008—it'll be an unfamiliar circumstance, but a familiar setting and a familiar foe.
UMass (15-3-3, 6-1-1 Atlantic 10) will return to Rudd Field to host Colgate (10-10-1, 4-1-1 Patriot League) for the second time this season, after the Minutemen took home a 2-1 win back on Sept. 16.
Thursday's rematch has infinitely more weight than that non-conference tilt in the early part of the season, and it will come down to two things—which team makes better adjustments from the initial meeting and which team has improved the most in the intervening time.
"I think both teams will have gotten better, it'll be a very interesting tie," said UMass coach Fran O'Leary. "We talk about getting better and we want to go out and prove to ourselves that our rate of improvement will be sufficient to get a result in this game. We know we will have to put on a better performance than we did against them a couple of months ago because they definitely have improved."
The Minutemen have certainly been in better form since that game; the win over Colgate in September was the start of an 11-match unbeaten run, and they're 12-2-1 overall since that win.
The Raiders, meanwhile, are 7-6-1 since that loss, which came during a brutal five-game losing streak in late September. Colgate, however, has been much better as of late, winning its last five en route to a Patriot League tournament championship.
The Raiders are a different team than the one UMass saw early in the fall, one with new tactics and playoff experience.
"They're going back to back in the tournament, so they're a very difficult opponent," O'Leary said. "We beat them at home early in the season but they've changed their lineup, they've changed their formation since then."
As far as O'Leary's concerned, it's a new season, and a new game.
"We're both new teams. I always feel that, come late in the season, you've put in 10 or 15 appearances, you're really a year older," O'Leary said. "So Davis [Smith] is really a sophomore, when he first played he was athletically a freshman, now he's really a sophomore. I don't think we can take a lot from that first game, it's an NCAA playoff game, they have more experience in it recently than we have, but we didn't have any experience going into the final four of the A-10, we'd never done that before, and we acquitted ourselves quite well."
The Minutemen have been excellent since taking a 1-0 loss to Dartmouth in September, on both ends of the pitch. An extremely impressive tournament run, in which they shut down three of the best offenses in the conference, has sparked a wave of confidence that they hope to ride into their first NCAA tournament appearance in nearly a decade.
"Right now we're peaking nicely," O'Leary said. "I think we've lost one of our last 14, and to go into games against these three teams [Fordham, Saint Louis and Virginia Commonwealth] and concede only one goal, we've proven that we can score goals over the course of the season, and what we've done lately is tighten considerably. You look at our team last year and we were very tight defensively, and maybe we didn't score enough goals, and if you look at the earlier part of the season we were scoring freely but maybe giving away some cheap goals. Now over the course of these three games we've really tightened, and that's helped us win the conference."
UMass has been the better team since the first meeting, but O'Leary says it'll come down to "who's better on the day," because in a single-elimination tournament, anything can happen.
Amin Touri can be reached at [email protected], and followed on Twitter @Amin_Touri.
difficult opponent
semifinalist
tournament championship
UMass Amherst Minutemen
Amin Touri, Editor in Chief
Amin Touri is the Editor in Chief of the Collegian. A senior, Touri is a journalism major with a concentration in sports journalism, and covers the men's...


Protect your data with secure document exchange.
Technology for secure document exchange is critical to protecting sensitive data from a wide variety of email security risks.
From financial records and customer information to intellectual property and future business plans, employees frequently need to share sensitive information via email, however, sending those files via secure emails can be a challenge. Traditional approaches to encryption — including enforced server-to-server Transport Layer Security or Public Key Infrastructure – often create administrative burden for senders and recipients alike. Some solutions mandate that require senders have knowledge of certificates and encryption keys and that recipients download and install specific software. When faced with this complexity, users may not always choose to use secure document exchange when sharing sensitive information, putting the data and the organization at risk.
Secure document exchange with Mimecast.
To simplify secure document exchange, a growing number of organizations are turning to Mimecast Secure Messaging, an easy-to-use secure messaging platform for sharing sensitive information with contacts outside the organization.
Mimecast's cloud-based email security, archiving and continuity services help to simplify email management and reduce the cost and complexity of protecting business email.
As a component of Mimecast's email security offerings, Mimecast Secure Messaging provides a user-friendly, secure channel for sending and receiving sensitive information and files through email. Users do not need any special knowledge encryption, and there are no client installation requirements for recipients.
How Mimecast's secure document exchange works.
To send a secure email or initiate a secure document exchange, users simply create a new email within Outlook for Windows or Mimecast for Mac, attach the desired documents, and choose a Send Secure option before clicking Send. Users may also choose from several secure email options to require read receipts, restrict printing and replying, or set expiration dates.
Once the message is sent, the email and attachments are uploaded to the secure Mimecast cloud where they are scanned for viruses, checked against data leak prevention policies and then stored in a secure AES encrypted archive.
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Learn more about secure document exchange with Mimecast, and about Mimecast solutions to prevent business email compromise and solve Office 365 email problems.


text:
<!DOCTYPE html>

    <meta charset="utf-8">
    <title>src/pixi/renderers/webgl/utils/WebGLGraphics.js - pixi.js</title>
    <link rel="stylesheet" href="http://yui.yahooapis.com/3.9.1/build/cssgrids/cssgrids-min.css">
    <link rel="stylesheet" href="../assets/vendor/prettify/prettify-min.css">
    <link rel="stylesheet" href="../assets/css/main.css" id="site_styles">
    <link rel="shortcut icon" type="image/png" href="../assets/favicon.png">

            API Docs for: 1.5.0

APIs

Classes

Modules

            <input type="search" id="api-filter" placeholder="Type to filter APIs">

AbstractFilter

AjaxRequest

AlphaMaskFilter

AssetLoader

AtlasLoader

autoDetectRenderer

BaseTexture

BitmapFontLoader

BitmapText

BlurFilter

CanvasGraphics

CanvasMaskManager

CanvasRenderer

CanvasTinter

Circle

ColorMatrixFilter

ColorStepFilter

DisplacementFilter

DisplayObject

DisplayObjectContainer

DotScreenFilter

Ellipse

EventTarget

FilterTexture

Graphics

GrayFilter

ImageLoader

InteractionData

InteractionManager

InvertFilter

JsonLoader

MovieClip

NormalMapFilter

PixelateFilter

PixiFastShader

PixiShader

Point

Polygon

PolyK

PrimitiveShader

Rectangle

Rope

SepiaFilter

Spine

Sprite

SpriteBatch

SpriteSheetLoader

Stage

Strip

Text

Texture

TilingSprite

TwistFilter

WebGLFilterManager

WebGLGraphics

WebGLMaskManager

WebGLRenderer

WebGLShaderManager

WebGLSpriteBatch

PIXI

        Show:

            <input type="checkbox" id="api-show-inherited" checked>
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            Private

            <input type="checkbox" id="api-show-deprecated">
            Deprecated

File: src/pixi/renderers/webgl/utils/WebGLGraphics.js

/**
 * @author Mat Groves http://matgroves.com/ @Doormat23
 */

/**
 * A set of functions used by the webGL renderer to draw the primitive graphics data
 *
 * @class WebGLGraphics
 * @private
 * @static
 */
PIXI.WebGLGraphics = function()
{

};

/**
 * Renders the graphics object
 *
 * @static
 * @private
 * @method renderGraphics
 * @param graphics {Graphics}
 * @param renderSession {Object}
 */
PIXI.WebGLGraphics.renderGraphics = function(graphics, renderSession)//projection, offset)
{
    var gl = renderSession.gl;
    var projection = renderSession.projection,
        offset = renderSession.offset,
        shader = renderSession.shaderManager.primitiveShader;

    if(!graphics._webGL[gl.id])graphics._webGL[gl.id] = {points:[], indices:[], lastIndex:0,
                                           buffer:gl.createBuffer(),
                                           indexBuffer:gl.createBuffer()};

    var webGL = graphics._webGL[gl.id];

    if(graphics.dirty)
    {
        graphics.dirty = false;

        if(graphics.clearDirty)
        {
            graphics.clearDirty = false;

            webGL.lastIndex = 0;
            webGL.points = [];
            webGL.indices = [];

        }

        PIXI.WebGLGraphics.updateGraphics(graphics, gl);
    }

    renderSession.shaderManager.activatePrimitiveShader();

    // This  could be speeded up for sure!

    // set the matrix transform
    gl.blendFunc(gl.ONE, gl.ONE_MINUS_SRC_ALPHA);

    gl.uniformMatrix3fv(shader.translationMatrix, false, graphics.worldTransform.toArray(true));

    gl.uniform2f(shader.projectionVector, projection.x, -projection.y);
    gl.uniform2f(shader.offsetVector, -offset.x, -offset.y);

    gl.uniform3fv(shader.tintColor, PIXI.hex2rgb(graphics.tint));

    gl.uniform1f(shader.alpha, graphics.worldAlpha);
    gl.bindBuffer(gl.ARRAY_BUFFER, webGL.buffer);

    gl.vertexAttribPointer(shader.aVertexPosition, 2, gl.FLOAT, false, 4 * 6, 0);
    gl.vertexAttribPointer(shader.colorAttribute, 4, gl.FLOAT, false,4 * 6, 2 * 4);

    // set the index buffer!
    gl.bindBuffer(gl.ELEMENT_ARRAY_BUFFER, webGL.indexBuffer);

    gl.drawElements(gl.TRIANGLE_STRIP,  webGL.indices.length, gl.UNSIGNED_SHORT, 0 );

    renderSession.shaderManager.deactivatePrimitiveShader();

    // return to default shader...
//  PIXI.activateShader(PIXI.defaultShader);
};

/**
 * Updates the graphics object
 *
 * @static
 * @private
 * @method updateGraphics
 * @param graphicsData {Graphics} The graphics object to update
 * @param gl {WebGLContext} the current WebGL drawing context
 */
PIXI.WebGLGraphics.updateGraphics = function(graphics, gl)
{
    var webGL = graphics._webGL[gl.id];

    for (var i = webGL.lastIndex; i < graphics.graphicsData.length; i++)
    {
        var data = graphics.graphicsData[i];

        if(data.type === PIXI.Graphics.POLY)
        {
            if(data.fill)
            {
                if(data.points.length>3)
                    PIXI.WebGLGraphics.buildPoly(data, webGL);
            }

            if(data.lineWidth > 0)
            {
                PIXI.WebGLGraphics.buildLine(data, webGL);
            }
        }
        else if(data.type === PIXI.Graphics.RECT)
        {
            PIXI.WebGLGraphics.buildRectangle(data, webGL);
        }
        else if(data.type === PIXI.Graphics.CIRC || data.type === PIXI.Graphics.ELIP)
        {
            PIXI.WebGLGraphics.buildCircle(data, webGL);
        }
    }

    webGL.lastIndex = graphics.graphicsData.length;

    webGL.glPoints = new Float32Array(webGL.points);

    gl.bindBuffer(gl.ARRAY_BUFFER, webGL.buffer);
    gl.bufferData(gl.ARRAY_BUFFER, webGL.glPoints, gl.STATIC_DRAW);

    webGL.glIndicies = new Uint16Array(webGL.indices);

    gl.bindBuffer(gl.ELEMENT_ARRAY_BUFFER, webGL.indexBuffer);
    gl.bufferData(gl.ELEMENT_ARRAY_BUFFER, webGL.glIndicies, gl.STATIC_DRAW);
};

/**
 * Builds a rectangle to draw
 *
 * @static
 * @private
 * @method buildRectangle
 * @param graphicsData {Graphics} The graphics object containing all the necessary properties
 * @param webGLData {Object}
 */
PIXI.WebGLGraphics.buildRectangle = function(graphicsData, webGLData)
{
    // --- //
    // need to convert points to a nice regular data
    //
    var rectData = graphicsData.points;
    var x = rectData[0];
    var y = rectData[1];
    var width = rectData[2];
    var height = rectData[3];

    if(graphicsData.fill)
    {
        var color = PIXI.hex2rgb(graphicsData.fillColor);
        var alpha = graphicsData.fillAlpha;

        var r = color[0] * alpha;
        var g = color[1] * alpha;
        var b = color[2] * alpha;

        var verts = webGLData.points;
        var indices = webGLData.indices;

        var vertPos = verts.length/6;

        // start
        verts.push(x, y);
        verts.push(r, g, b, alpha);

        verts.push(x + width, y);
        verts.push(r, g, b, alpha);

        verts.push(x , y + height);
        verts.push(r, g, b, alpha);

        verts.push(x + width, y + height);
        verts.push(r, g, b, alpha);

        // insert 2 dead triangles..
        indices.push(vertPos, vertPos, vertPos+1, vertPos+2, vertPos+3, vertPos+3);
    }

    if(graphicsData.lineWidth)
    {
        var tempPoints = graphicsData.points;

        graphicsData.points = [x, y,
                  x + width, y,
                  x + width, y + height,
                  x, y + height,
                  x, y];

        PIXI.WebGLGraphics.buildLine(graphicsData, webGLData);

        graphicsData.points = tempPoints;
    }
};

/**
 * Builds a circle to draw
 *
 * @static
 * @private
 * @method buildCircle
 * @param graphicsData {Graphics} The graphics object to draw
 * @param webGLData {Object}
 */
PIXI.WebGLGraphics.buildCircle = function(graphicsData, webGLData)
{

    // need to convert points to a nice regular data
    var rectData = graphicsData.points;
    var x = rectData[0];
    var y = rectData[1];
    var width = rectData[2];
    var height = rectData[3];

    var totalSegs = 40;
    var seg = (Math.PI * 2) / totalSegs ;

    var i = 0;

    if(graphicsData.fill)
    {
        var color = PIXI.hex2rgb(graphicsData.fillColor);
        var alpha = graphicsData.fillAlpha;

        var r = color[0] * alpha;
        var g = color[1] * alpha;
        var b = color[2] * alpha;

        var verts = webGLData.points;
        var indices = webGLData.indices;

        var vecPos = verts.length/6;

        indices.push(vecPos);

        for (i = 0; i < totalSegs + 1 ; i++)
        {
            verts.push(x,y, r, g, b, alpha);

            verts.push(x + Math.sin(seg * i) * width,
                       y + Math.cos(seg * i) * height,
                       r, g, b, alpha);

            indices.push(vecPos++, vecPos++);
        }

        indices.push(vecPos-1);
    }

    if(graphicsData.lineWidth)
    {
        var tempPoints = graphicsData.points;

        graphicsData.points = [];

        for (i = 0; i < totalSegs + 1; i++)
        {
            graphicsData.points.push(x + Math.sin(seg * i) * width,
                                     y + Math.cos(seg * i) * height);
        }

        PIXI.WebGLGraphics.buildLine(graphicsData, webGLData);

        graphicsData.points = tempPoints;
    }
};

/**
 * Builds a line to draw
 *
 * @static
 * @private
 * @method buildLine
 * @param graphicsData {Graphics} The graphics object containing all the necessary properties
 * @param webGLData {Object}
 */
PIXI.WebGLGraphics.buildLine = function(graphicsData, webGLData)
{
    // TODO OPTIMISE!
    var i = 0;

    var points = graphicsData.points;
    if(points.length === 0)return;

    // if the line width is an odd number add 0.5 to align to a whole pixel
    if(graphicsData.lineWidth%2)
    {
        for (i = 0; i < points.length; i++) {
            points[i] += 0.5;
        }
    }

    // get first and last point.. figure out the middle!
    var firstPoint = new PIXI.Point( points[0], points[1] );
    var lastPoint = new PIXI.Point( points[points.length - 2], points[points.length - 1] );

    // if the first point is the last point - gonna have issues :)
    if(firstPoint.x === lastPoint.x && firstPoint.y === lastPoint.y)
    {
        points.pop();
        points.pop();

        lastPoint = new PIXI.Point( points[points.length - 2], points[points.length - 1] );

        var midPointX = lastPoint.x + (firstPoint.x - lastPoint.x) *0.5;
        var midPointY = lastPoint.y + (firstPoint.y - lastPoint.y) *0.5;

        points.unshift(midPointX, midPointY);
        points.push(midPointX, midPointY);
    }

    var verts = webGLData.points;
    var indices = webGLData.indices;
    var length = points.length / 2;
    var indexCount = points.length;
    var indexStart = verts.length/6;

    // DRAW the Line
    var width = graphicsData.lineWidth / 2;

    // sort color
    var color = PIXI.hex2rgb(graphicsData.lineColor);
    var alpha = graphicsData.lineAlpha;
    var r = color[0] * alpha;
    var g = color[1] * alpha;
    var b = color[2] * alpha;

    var px, py, p1x, p1y, p2x, p2y, p3x, p3y;
    var perpx, perpy, perp2x, perp2y, perp3x, perp3y;
    var a1, b1, c1, a2, b2, c2;
    var denom, pdist, dist;

    p1x = points[0];
    p1y = points[1];

    p2x = points[2];
    p2y = points[3];

    perpx = -(p1y - p2y);
    perpy =  p1x - p2x;

    dist = Math.sqrt(perpx*perpx + perpy*perpy);

    perpx /= dist;
    perpy /= dist;
    perpx *= width;
    perpy *= width;

    // start
    verts.push(p1x - perpx , p1y - perpy,
                r, g, b, alpha);

    verts.push(p1x + perpx , p1y + perpy,
                r, g, b, alpha);

    for (i = 1; i < length-1; i++)
    {
        p1x = points[(i-1)*2];
        p1y = points[(i-1)*2 + 1];

        p2x = points[(i)*2];
        p2y = points[(i)*2 + 1];

        p3x = points[(i+1)*2];
        p3y = points[(i+1)*2 + 1];

        perpx = -(p1y - p2y);
        perpy = p1x - p2x;

        dist = Math.sqrt(perpx*perpx + perpy*perpy);
        perpx /= dist;
        perpy /= dist;
        perpx *= width;
        perpy *= width;

        perp2x = -(p2y - p3y);
        perp2y = p2x - p3x;

        dist = Math.sqrt(perp2x*perp2x + perp2y*perp2y);
        perp2x /= dist;
        perp2y /= dist;
        perp2x *= width;
        perp2y *= width;

        a1 = (-perpy + p1y) - (-perpy + p2y);
        b1 = (-perpx + p2x) - (-perpx + p1x);
        c1 = (-perpx + p1x) * (-perpy + p2y) - (-perpx + p2x) * (-perpy + p1y);
        a2 = (-perp2y + p3y) - (-perp2y + p2y);
        b2 = (-perp2x + p2x) - (-perp2x + p3x);
        c2 = (-perp2x + p3x) * (-perp2y + p2y) - (-perp2x + p2x) * (-perp2y + p3y);

        denom = a1*b2 - a2*b1;

        if(Math.abs(denom) < 0.1 )
        {

            denom+=10.1;
            verts.push(p2x - perpx , p2y - perpy,
                r, g, b, alpha);

            verts.push(p2x + perpx , p2y + perpy,
                r, g, b, alpha);

            continue;
        }

        px = (b1*c2 - b2*c1)/denom;
        py = (a2*c1 - a1*c2)/denom;

        pdist = (px -p2x) * (px -p2x) + (py -p2y) + (py -p2y);

        if(pdist > 140 * 140)
        {
            perp3x = perpx - perp2x;
            perp3y = perpy - perp2y;

            dist = Math.sqrt(perp3x*perp3x + perp3y*perp3y);
            perp3x /= dist;
            perp3y /= dist;
            perp3x *= width;
            perp3y *= width;

            verts.push(p2x - perp3x, p2y -perp3y);
            verts.push(r, g, b, alpha);

            verts.push(p2x + perp3x, p2y +perp3y);
            verts.push(r, g, b, alpha);

            verts.push(p2x - perp3x, p2y -perp3y);
            verts.push(r, g, b, alpha);

            indexCount++;
        }
        else
        {

            verts.push(px , py);
            verts.push(r, g, b, alpha);

            verts.push(p2x - (px-p2x), p2y - (py - p2y));
            verts.push(r, g, b, alpha);
        }
    }

    p1x = points[(length-2)*2];
    p1y = points[(length-2)*2 + 1];

    p2x = points[(length-1)*2];
    p2y = points[(length-1)*2 + 1];

    perpx = -(p1y - p2y);
    perpy = p1x - p2x;

    dist = Math.sqrt(perpx*perpx + perpy*perpy);
    perpx /= dist;
    perpy /= dist;
    perpx *= width;
    perpy *= width;

    verts.push(p2x - perpx , p2y - perpy);
    verts.push(r, g, b, alpha);

    verts.push(p2x + perpx , p2y + perpy);
    verts.push(r, g, b, alpha);

    indices.push(indexStart);

    for (i = 0; i < indexCount; i++)
    {
        indices.push(indexStart++);
    }

    indices.push(indexStart-1);
};

/**
 * Builds a polygon to draw
 *
 * @static
 * @private
 * @method buildPoly
 * @param graphicsData {Graphics} The graphics object containing all the necessary properties
 * @param webGLData {Object}
 */
PIXI.WebGLGraphics.buildPoly = function(graphicsData, webGLData)
{
    var points = graphicsData.points;
    if(points.length < 6)return;

    // get first and last point.. figure out the middle!
    var verts = webGLData.points;
    var indices = webGLData.indices;

    var length = points.length / 2;

    // sort color
    var color = PIXI.hex2rgb(graphicsData.fillColor);
    var alpha = graphicsData.fillAlpha;
    var r = color[0] * alpha;
    var g = color[1] * alpha;
    var b = color[2] * alpha;

    var triangles = PIXI.PolyK.Triangulate(points);

    var vertPos = verts.length / 6;

    var i = 0;

    for (i = 0; i < triangles.length; i+=3)
    {
        indices.push(triangles[i] + vertPos);
        indices.push(triangles[i] + vertPos);
        indices.push(triangles[i+1] + vertPos);
        indices.push(triangles[i+2] +vertPos);
        indices.push(triangles[i+2] + vertPos);
    }

    for (i = 0; i < length; i++)
    {
        verts.push(points[i * 2], points[i * 2 + 1],
                   r, g, b, alpha);
    }
};


text:
Where Can I Bet on NASCAR Races Online?
You can bet on NASCAR races over the Internet at a number of online sportsbook sites. Not all offer the same great betting options however, nor the same top signup bonuses for that matter.
With NASCAR betting, the two most popular options are wagering on a driver to win the race and the individual head-to-head race matchups.
How To Bet On NASCAR
If you're betting on NASCAR, there are two main options for it. The first is to predict the winner of the race. If you go that route, you'll see odds of +250, +500, +1500 and all those mean is that if you bet $100, you'll win the amount after the plus sign.
Now you can also bet on head-to-head matchups in NASCAR. What this means is when there are two drives pitted against each other by the odds makers, you decide which driver you think will have the better finish. They don't have to win the race outright but they do have to finish ahead of the driver you are betting against.
BetDSI.com offers some excellent betting options on NASCAR races.
Where Can I Watch, Bet the McGregor vs. Poirier Fight UFC 257 From Anaheim
Betting on UFC 257 from Anaheim is available via BetUS, which offers a generous welcome bonus (max bonus $3125) and has been in business since 1994
Where Can I Watch, Bet the McGregor vs. Poirier Fight UFC 257 From Anchorage
Peanut Farm and 907 Ale House & Grill are two of the venues showing UFC 257
Where Can I Watch, Bet the McGregor vs. Poirier Fight UFC 257 From San Jose, California
Betting on UFC 257 from San Jose, CA is available via BetUS, which offers a generous welcome bonus (max bonus $3125) . Scroll down to find out where to watch this fight from the San Jose, CA area.
Where Can I Watch, Bet the McGregor vs. Poirier Fight UFC 257 From San Diego
Betting on UFC 257 from San Diego is available via BetUS, which offers a generous welcome bonus (max bonus $3125) . Scroll down to find out where to watch this fight from the San Diego area.
Where Can I Watch, Bet the McGregor vs. Poirier Fight UFC 257 From LA
Betting on UFC 257 from LA is available via Jazz Sports, which offers a generous welcome bonus (max bonus $1000) PLUS a $25 FREE bet and has been in business since 1994. While LA is getting hit hard by the coronavirus, forcing most restaurants and bars to shutter, there are options outside the city.


Image: How times change: the Parish Council's listed Grade II phone box in Bridge Street, restored by Wye Ground Force, is now a source of local information for visitors to Wye.
Please get in touch by email, or register for e-newsletters via the form below. Alternatively, write to the Parish Council's office address, or leave a note for the Parish Clerk in the free post box in Wye News.
Please supply this if you require a response.
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The Parish Council needs your postcode to confirm that you are a real person, and not a robot.
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The Parish Council needs your home address and postcode to confirm that you are a real person, not a robot.
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text:
Irreversible Electroporation in Patients With Liver Tumours: Treated-area Patterns With Contrast-enhanced Ultrasound
Comments Off on Irreversible Electroporation in Patients With Liver Tumours: Treated-area Patterns With Contrast-enhanced Ultrasound
IRE has been gaining increasing interest because the non-thermal properties of this method[9] permit the ability to ablate tumours adjacent to vital structures[10]. Previous studies have demonstrated that US findings after IRE application in the liver evolve sequentially over time, from seconds to at least hours[3, 11, 12]. Our results show the evolution of post-IRE ablation patterns over the clinically relevant time period.
As noted in an animal-based experiment, a strong association exists between conventional US and histopathology[5]. In our study, on conventional US, IRE ablation zones of most patients appear as a developing hypo-echoic area that demonstrates an increasingly hyperechogenic ablation zone starting one day after the procedure.
Our US findings after IRE ablation evolved sequentially over time. The findings showed good correlation with those in previous studies[5, 13]. In the study, specimens obtained immediately after ablation showed that the widened oedematous sinusoidal spaces were filled mainly by fluid, and very little haemorrhagic infiltrate was observed. As time passed, the haemorrhagic infiltrate became more dominant, which might be due to the widened fluid-filled sinusoids at the beginning of the procedure. The authors attribute this hyper-echogenicity to red blood cell accumulation over time. The degree of red blood cell infiltrate was qualitatively associated with echogenicity. Lee et al also reported the US findings of 55 ablation zones immediately and 1 day after ablation and showed that the immediate hypo-echogenicity transformed to total hyper-echogenicity in the treatment zone 1 day after the procedure[13]. Appelbaum et al speculated that red blood cells progressively infiltrated into deep regions of the ablated zone so that the hyper-echoic rim on US at 90–120 minutes transitioned to complete hyper-echogenicity within 24 hours[5]. There is concordance between our findings and those of previous studies that described the characteristics of images obtained after ablation.
In CEUS, most of the ablated zones showed hypo-enhancement immediately after IRE. Chung et al found the following zones with different enhancement patterns on CT perfusion images in normal porcine liver: an inner non-enhanced zone; a middle well-defined progressive internal enhancement zone, and an outer ill-defined arterial enhancement zone. On histopathology, the inner and middle zones accounted for the extent of cell death[14]. The histological examination suggested that the apoptotic process was involved with complete cell death in the pathophysiology of cell death caused by IRE.
The CEUS images of the IRE ablation zones in normal liver tissue differed from the images of liver tumours treated with IRE. Our study also found that 10 ablated zones appeared with hypo-enhancement immediately after IRE but became non-enhanced one day after IRE, which is due to diverse reasons. Lee et al attributed the focal hyper-attenuation to the release of contrast medium into an ablation defect caused by an IRE-induced microvasculature leakage within the defect zone[15]. Because the zones became non-enhanced on the follow-up CEUS images, the hyper-enhancement was probably caused by extraluminal contrast material. Another opinion is about the differences in contrast agent concentrations. Guo et al suggested that nanometre-scale pores in the tissue cell membrane caused contrast agent to accumulate in the IRE zone and allowed for the contrast agent to be internalized into the intracellular environment rather than remaining extracellularly[16], which makes evaluating whether the viable tissue is a residual tumour difficult after ablation. Therefore, follow-up CEUS is necessary to assess the viable portion. However, unlike normal regeneration activity, the residual tumour can continue growing and results in a newly enhanced region.
Most of the non-enhancement pattern on CEUS 1 month after ablation is a sign of effective IRE treatment, besides there are still false negatives. Such non-enhancement patterns are different to those of the thermal ablation zone after complete ablation. Previous histologic examinations of the ablation zones showed cell death caused by apoptosis[13]. Cell death is seen with full preservation of the peri-ablative zone structures, such as blood vessels and bile ducts.
In the present study, only one patient continuously showed an enhanced ablation zone immediately and on follow-up CEUS images. The ablation zone became hyper-enhanced during the early arterial phase, slightly wash out in the late arterial phase and presented as hypo-enhanced in the late phase. To elucidate the reason for this pattern, the patient underwent a liver biopsy one month after IRE. The physiology results showed small patchy necrosis, inflammatory fibrosis tissue hyperplasia and foam cell aggregation. The result ruled out the possibility of recurrence. A reasonable explanation for this finding is hyperplasia of the inflammatory tissue. This result can cause confusion in clinical practice. Therefore, sequential follow-up is essential. Further investigation is needed to study the histological and cytological mechanisms underlying this process.
In our study, only 2 ablation zones still appeared as hypo-echoic areas, and both zones were in the same patient. After 1 month of follow-up, recurrence occurred near one of the zones treated with IRE ablation. In a previous multi-institutional review from 2009 through 2012, 31% of the patients had recurrence during a median follow-up of 18 months. Of the total 31% of patients with recurrence, 10.7% had local recurrences at the ablated site[4]. Previous work attributed these recurrences to electric field sinks that resulted from the heterogeneous structure and conductivity of the liver[17]. Later work from the authors indicated that the IRE-treated extracellular matrix (ECM) provides an environment for the activation and differentiation of progenitor cells[18], but the mechanism is not completely understood; in contrast, some studies have suggested that abnormal ECM affects cancer progression by directly promoting cellular transformation and metastasis and facilitating tumour-associated angiogenesis and inflammation, leading to the generation of a tumorigenic microenvironment[19]. The role of the IRE-spared tumour matrix in follow-up recurrences requires further research. Another theory is about the size of the treated liver tumours. Niessen et al found that large tumour volumes (> 5 cm3) portended early local recurrence[20].
In our study, the intra-hepatic blood vessels and bile duct remained almost completely intact after IRE. The hepatohilar bile duct of only one patient showed an unclear contrast agent pattern immediately after IRE. After 15 minutes, the phenomenon disappeared. However, a consensus on the mechanism of IRE has not yet been realized. This effect could be due to the high proportion of collagenous connective tissue. A further hypothesis is that the gap junctions, which are present in large numbers in the muscularis propria of the blood vessels and the bile duct walls, could act as a conductive structure for the electrical currents; thus, the current can be passed from cell to cell without leading to destruction of the cell membrane[14]. Whether the effects of IRE are caused by a thermal or non-thermal mechanism remains unclear.
This study has several limitations. First, our study had a small sample size for the span of more than 2 years. Another limitation was that almost all of the patients we included in our study group previously underwent right or left liver resection and thermal ablation or catheter chemical ablation. The origin of the ablation zones was heterogeneous. However, this circumstance mirrors the status of our clinical treatment strategies. IRE as a novel technique and was not the first choice in our hospital. Only patients who experienced tumour recurrence after liver resection and thermal ablation were considered for IRE. Because of this situation, assessing the images of the ablated zones during subsequent follow-up imaging examinations is important. We conclude that CEUS may be a useful tool for assessing the characteristics of post-IRE ablation changes. And it is an effective way to evaluate the therapeutic efficacy 1 month after ablation. Further studies are needed to evaluate more patients to precisely depict the appearance of hepatic zones on CEUS.
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text:
Road Tapes, Venue #2 es un álbum póstumo de Frank Zappa, el cual fue publicado en noviembre de 2013. Hay canciones de tres conciertos, todo ellos celebrados en agosto de 1973. Esta colección, con una duración de más de dos horas, da la experiencia de un concierto entero.  Esta es el lanzamiento oficial número 96.

Lista de canciones
Todas las canciones escritas por Frank Zappa

Disco 1:

Disco 2:

Lista de artistas
 Frank Zappa – guitarra, voces
 Jean-Luc Ponty – violín eléctrico
 George Duke – teclados, voces
 Ian Underwood – sintetizador, instrumentos de viento - madera
 Ruth Underwood – percusión
 Bruce Fowler – tromboón
 Tom Fowler – bajo
 Ralph Humphrey – batería

Referencias

Frank Zappa
Álbumes de Estados Unidos de 2013
Álbumes en vivo de 2013
Álbumes en vivo de 1973
Álbumes de Frank Zappa
Álbumes póstumos

redpajama_set_name: RedPajamaWikipedia


Find places to eat in East Rutherford, New Jersey: restaurants, fast foods, pizza, barbecues, coffee shops.
East Rutherford map with restaurants locations is the best place to discover restaurant, pizza, barbecue, grill or coffee shop locations. It helps you to quickly find your preferred place for taking your breakfast, lunch or dining.
Tags: East Rutherford restaurant, East Rutherford pizza, East Rutherford coffee shop .


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Q: Storing data in Riak with automatic ID? If I make a HTTP POST to riak, i.e http://localhost:8098/riak/mybucket along with JSON-encoded data {name: "John Doe"}, the object is saved as expected.
However, this data will be assigned to an id set by Riak automatically, something like WAqRNgxZl10FK0F3FLuorByNHgN.
Is it possible to make Riak return this id in the response of the HTTP POST?

A: According to the Riak documentation, it returns the new key/ID in the Location header.

In the output, the Location header will give the you key for that
  object. To view the newly created object, go to
  "http://127.0.0.1:8091/Location" in your browser.

You can see the docs here - Scroll down to "Store a new object and assign random key "


Today's Diesel price in Rudrapur (Uttarakhand) is Rs. 65.49 per Litre. Last change in Rudrapur diesel price was on April 25, 2019 and it was increased by +0.07 rupees. In addition, we bring you the most recent diesel price changes in Rudrapur city. The diesel price is inclusive of Uttarakhand state taxes.


When the Royal Shakespeare Company decided to run its production of Julius Caesar at the Noël Coward Theatre (it's already been a hit in Stratford-upon-Avon) it knew one thing: the afterparty of the opening night had to be good. Really, really good. Tell-your-grandchildren good. And it was! Hurrah! After watching the show (it's completely brilliant and running until September 15th as part of the World Shakespeare Festival), everyone sauntered to Salvador and Amanda's for champagne, Spanish wine and a joyfully endless procession of tapas. While Yasmin and Tallulah Le Bon nattered to Paul Sculfor, Rosario Dawson chatted to Ray Fearon and Chucky Venn and Nick Moran said hello to Lenora Crichlow. Then The Vibes of March started their set (the band also plays during the show) and everyone danced - not unexpectedly - until 2am.


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Il monte Katmai è un vulcano degli Stati Uniti situato in Alaska, nel parco nazionale e riserva di Katmai. Questa montagna è coronata da una caldera contenente un lago formatasi durante l'eruzione del 1912, l'unica conosciuta di questo vulcano.

Geografia
Il monte Katmai si trova nel sud-ovest della Alaska, nella penisola di Alaska. Il vulcano è circondato dal Novarupta ad ovest, e dalla valle dei Diecimila Fumi a nord-ovest, dal Snowy nel nord-est, dalla baia di Kukak ad est, dallo stretto di Šelichov ad est, sud-est e sud.

La cima della montagna è coronata da una caldera ampia tre chilometri per quattro di lunghezza; uno dei suoi bordi s'innalza a 2.047 metri sul livello del mare. La caldera contiene un lago profondo 250 metri che ha completamente sommerso un'antica isola, composta da un duomo di lava formatosi nel 1916, quattro anni dopo l'eruzione che ha creato la caldera. I pendii della montagna sono coperti da ghiacciai.

Tecnologia
Katmai è anche il nome in codice della tecnologia alla base della prima generazione di processori Pentium III.

Note

Bibliografia
 Erskine, Wilson Fiske. (1965). Katmai. A narrative of the eruption of June 1912 and its effects on the town of Kodiak and its community, taken from letters, diaries and notes written at the time. London, New York and Toronto: Abelard-Schuman.
 Hildreth, W., J. Fierstein, and J.E. Robinson. (2003). Geologic map of the Katmai Volcanic Cluster, Katmai National Park, Alaska, Geologic Investigations Series Map I-2778. Reston, VA: U.S. Department of the Interior, U.S. Geological Survey.

Altri progetti

Collegamenti esterni
 Alaska Volcano Observatory: Katmai

Katmai


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home Lifestyle Cole Hauser's Kids: Learn About His Family Life
Cole Hauser's Kids: Learn About His Family Life
Published Mon Sep 13 2021 By shirayoky
Cole Hauser's Kids and Married Life: The Actor Is a Father to three children!
Cole Kenneth Hauser is an actor. He is renowned for his roles in Higher Learning, School Ties, Dazed, and Confused, Good Will Hunting, Pitch Black, Tigerland, Hart's War, Tears of the Sun, The Family that Preys, and Fast and Furious.
On March 22, 1975, Cole was born in Santa Barbara, California, to Cass Warner, founded the film production company Warner Sisters and actor Wings, Hauser. Cole is of Irish and German descent on his father's side and Jewish on his mother's.
Cole stars as a ranch alongside ranch owner and family patriarch John Dutton (Kevin Costner) on the Paramount Network show. A steamy romantic relationship with Dutton's daughter, Beth (Kelly Reilly), often leaves fans overwhelmed and might make us wonder if Hauser is married in real life. Continue reading to know more.
Cole Hauser Shares Three Kids with His Wife!
Cole is happily married to actress and photographer Cynthia Daniel. Daniel stepped down from acting in 2002, started chasing a career in photography, and opened her own business, Five Arrows Photography. They tied the knot in 2006 and shared three lovely children.
Cole Hauser enjoys a blissful life with his wife and kids.
Photo Source: Throwbacks
Before their marriage, they welcomed their first child together, Ryland Hauser, in 2004. After four years later, they welcomed their second child, Colt Daniel Hauser, and Steely Rose, their third child, daughter, in the time frame of 2013.
Related: Norman Reedus's Kids: Learn About His Family Life.
Did Cole Hauser and Kelly Reilly Accidentally Confirm Beth Dutton Survived the Season 3 Finale?
Yellowstone Season 3 presented an explosive ending that imprinted the fate of three Dutton family members in the series. John (Kevin Costner), Beth (Kelly Reilly), Dutton, and Kayce (Luke Grimes) were ambushed. As the last episode aired in August 2020, fans have been trying to find out the clues as to who could still be alive. To quench the curiosity, Cole Hauser (Rip Wheeler) and Reilly gave an interview ahead of season 4.
Fans speculated on the possibility that the on-screen couple just accidentally confirmed that Beth survived? Yellowstone star Cole Hauser says Beth is the other half of Rip's life. Also, in the discussion, Cole pointed out that Beth is Rip's one and only one love.
How Yellowstone's Cole Hauser Thinks Beth And Rip's Relationship.
Photo Source: Cinema Blend
"As far as Rip's concerned, that was his first and only love from when he was 15 years old," Cole acclaimed. "Time eventually stopped for him and gave relization how special she was and what she could give to his life. But he has lost her a lot over time."
It's interesting to note in Hauser's particular comment in specific the "four years" part. Logically it generally means four seasons equals too four years. Nevertheless, if that's the case, it represents that Cole confirmed Beth, who will survive the season 3 finale ambush.
Don't miss out: Alvaro Morte's Kids: Learn About His Family Life.
Rip and Beth's romance seems slightly not over yet. Reilly acclaimed that viewers see Rip and Beth interrelate with all of the other characters on Yellowstone. However, when they are engulfed simultaneously, "The Duo just bring out a whole different color in each other."
"It provides a level of ease for Beth, a place for her to rest and lay down her weapons," Reilly pointed out. "Rip loves her in a way that's so unconditional and she's starting to settle into that place. It's so beautiful these broken characters are finding some sort of home with each other."
For more information and news on your favorite stars, stay connected to Glamour Fame.