For the past few months, ViralGains' Business Development Associate Neil Aronson has conducted extensive research on the Hispanic Advertising Market. His presentation last week inspired ViralGains to focus on learning more about this market segment and its involvement with online video.
Hispanics have demonstrated their appreciation for original Hispanic content—which is often in Spanish, English or both—by responding positively to the material. According to an article by comSource, Hispanic-specific ads are "three times as effective as ads dubbed into Spanish." If brands can create video content that is specifically tailored to the Hispanic market, it will be easier to not only reach, but also engage this audience.
Earlier in May, McDonald's was awarded Marketer of the Year by AHAA: The Voice of Hispanic Marketing. McDonald's worked with U.S. Hispanic agency Alma and succeeded in creating connections with Hispanic audiences by incorporating popular Hispanic themes like community, family and traditions. Hard work, pride and strong family values are represented in the company's spot "First Customer". Another campaign produced by Alma and McDonald's titled "Cancha," features camaraderie and soccer, a Hispanic tradition.
Neil informed us of the differences in Spanish usage depending on age and generation. AOL's Hispanic Cyberstudy presents three main categories for marketers to divide Hispanics into: Spanish-dominant, bilingual, and English-dominant. The McDonald's commercial "First Customer" contains a mixture of Spanish and English as it is predominantly for a bilingual Hispanic audience. However, the "Cancha" ad was filmed almost completely in Spanish with only the tagline 'I'm loving it' in English. This approach is inclusive of all categories but focuses on Spanish-dominant Hispanics.
Salter believes that this is the future of advertising as it integrates the growing Hispanic population as well as general audiences in major networks.
Advertisers can use these categories of Spanish usage and language mixtures to create content that will directly appeal to the desired market. Due to the variety of ways brands can target the Hispanic market based on language categories and popular Hispanic themes, branded video content is an ideal marketing tool.
The Miami Herald recently published an article presenting multiple "mainstream companies" whose marketing trends are being set by Latinos, including Google. The article reinforced Neil's information on Hispanics and their love for online video and social media.
Hispanics are "four times more likely to share branded content such as videos and commercials through social media, [and] are driving trends on digital and mobile devices". With the desire and passion that Hispanics have demonstrated for sharing branded content, brands and marketers can easily increase their reach within this market.
In order for this content to be shared, it must be accessible to Hispanics. Most Hispanics use mobile devices to access the Internet. According to a study by Google and OTX, U.S. Hispanics are significantly more likely to have a smartphone than the general population (45% v. 34%). Younger generations have been introduced to the Internet via smartphones as they are more affordable and portable than computers or laptops. These devices allow advertisers to reach a wider audience and provide more channels through which viewers can consume online video.
When it comes to online video campaigns, create content that is relatable to Hispanic audiences—Hispanics identify with values like community, family and typical traditions. To really have a personalized and authentic feeling, video content should be in Spanish or a mixture of Spanish and English and more importantly, it must be accessible on mobile devices to drive social sharing.


text:
Compulsions to lie to their people: MEA on Pak's ICJ claims
Sehwag breaks silence on Dhoni's retirement rumours
I live the most regular life: Spider-Man: Far From Home actor Tom Holland
Updated Jun 26, 2019 | 16:15 IST | IANS
Sharing insights of his personal life, Tom Holland said that when he is away from the show business, he lives a normal and regular life. He said that he keeps his family close so that they can correct him.
Tom Holland | Photo Credit: IANS
Bali: It has been a crazy ride to fame for Tom Holland, who is winning hearts all around the world as the new Spider-Man. But he does not want to get lost in the glitz and glamour of the industry.
The actor thinks he has done a great job at evading the spotlight and says he lives the "most normal and regular life ever".
"I have done quite a good job of only being in the spotlight when I need to be... Like I don't get paparazzied. I don't go to fancy parties. I don't do that kind of stuff," Holland said in an interview while promoting his film Spider-Man: Far From Home here.
"When I am not on the press tour or doing red carpet, I live the most normal and regular life ever. I have done a good job, at kind of, keeping out of the spotlight when it is possible," he added.
How important it is to stay away from the limelight?
"It is very important because you can get lost in it. No one will ever say no (to you) and no one will ever tell you anything bad. That is why I keep my brothers, my family very close because they will tell me that 'I am being a d*ck or an idiot'," the 23-year-old said.
"So, it is super important and I try very hard to keep away from it. And that is why when I am not on the press tour, you will never see me in the newspaper or on a tabloid because I am at home playing golf," added the actor, who has three brothers -- Sam, Paddy and Harry.
The London native says working and travelling back-to-back can get "lonely", and being with family helps him deal with it well.
"What is great is that they (family members) don't tag along because Harry works (with me). He is a videographer. And we are actually planning to direct our film this year, which is exciting.
"Sam sleeps in his hotel room... He is on a holiday here," he said with a chuckle.
On a serious note, he said: "It is lovely to be able to share this process because it will be quite lonely otherwise. I spend so much time on the road."
For Holland, the path towards showbiz began getting carved when he was a child. The son of English comedian Dominic Holland studied dance when he was in school, and went on to do Billy Elliot The Musical.
He featured in films like The Impossible, How I Live Now, In The Heart of the Sea and The Lost City of Z. But his big ticket to Hollywood came with role as the iconic web-slinger.
Holland was introduced as Spider-Man in Captain America: Civil War in 2016. He got his first solo movie with Spider-Man: Homecoming -- which took the superhero back to school.
He will be back as the superhero with his second solo movie Spider-Man: Far From Home, which Sony Pictures Entertainment India will release in India on July 4 in English, Hindi, Tamil and Telugu.
The actor might not be a superhero or the 'friendly neighbourhood Spider-Man' in real life, but he came across as a friendly and affable person with a charming personality -- with the way he cracked jokes in the middle of the interview, by taking a jibe at his track record of giving out spoilers and a little panic attack when he was unable to find his phone in his pocket.
Looking back at his journey, he said: "It has been crazy man. Spider-Man: Homecoming was a whirlwind, and the press tour was crazy. And since then I haven't stopped. I have been lucky that I have been making movies and working with people who I really admire."
He says the ride in showbiz has so far been fun, but a "little tiring" as well.
"I have learnt this year that sometimes working too much leads to doing bad work. I am kind of learning to take a little bit of break and look after myself a little bit better."
Complete your TV viewing experience with the best of Hollywood entertainment and News. Get the Times Movies And News pack at just Rs 13. Ask your cable/DTH provider for Times M.A.N. pack now. Know more
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I live the most regular life: Spider-Man: Far From Home actor Tom Holland Description: Sharing insights of his personal life, Tom Holland said that when he is away from the show business, he lives a normal and regular life. He said that he keeps his family close so that they can correct him. Times Now

redpajama_set_name: RedPajamaCommonCrawl


text:
Kevin (nee-McCall) Guyette
November 8, 1953 - October 27, 2018
Executive Director for the Foundation of ARC in Warren County
In Lieu of Flowers: Donations can be made in her memory to the Humane Society or any charitable cause you believe would benefit from
Obituaries » Kevin (nee-McCall) Guyette
Kevin (nee-McCall) Guyette, 64, of Mt. Arlington NJ, passed away very peacefully at her home on Oct. 27, 2018.
Kevin was born Nov. 8, 1953 and she was raised in Denville NJ by her parents June and William McCall with her three siblings Willie, Katie, and Eileen.
She will be missed by many. Kevin was a compassionate, generous anomaly with an unyielding moral compass that endeared her to everyone lucky enough to know her. Kevin is a proud mother of two sons, Stephen and Michael, and is loved by scores of friends, many of which so close they consider her family.
Kevin committed her life to providing resources, furthering community engagement and helping under served members of our community as the Executive Director for the Foundation of ARC in Warren County and as an active member of Rotary.
Celebration of life gathering will be held on Thursday, Nov. 8th, her birthday, at the Panther Valley Golf and Country Club. 5:30 p.m. – 7:30 p.m. at 1 Forest Road, Allamuchy Township, NJ 07820.
In lieu of flowers, donations can be made in her memory to the Humane Society or any charitable cause you believe could benefit.


Our fun, relaxed dining experience where Executive Chef Blake Seymour has an exceptional local seafood menu. Blake's menu will be a share seafood feast that includes several courses plus dessert. For the non-seafood lovers, please let us know upon booking and we will provide an alternate option. Always a wonderful dining experience.


validated nameId is compared to the name/email.
# Copyright and license info is available in the LICENSE file.
# the work around is that the agent adds a header for the pertinent data.
"""Build out the settings for SAML library."""
# is expecting, and has the correct IdP certificate.
# to the installation location of the pysaml module.
"""Build a fake request object for python3-saml to use."""
"""Produce a base64 encoded version of name_id."""
"""Load the previously saved request identifier for this user."""
"""Save the JSON formatted cookies to a file."""
"""Save the SAML session index for the logout trigger to use."""
"""Read the SAML response and verify user match."""
# Read the SAML response from standard input.
# a quick sanity check to avoid getting an odd exception.
#5 25196 nathan_fiedler Retry and then raise the error if unsuccesful.
#4 25195 nathan_fiedler Retry IdP metadata fetch a couple of times.
#2 24933 nathan_fiedler Add copyright and license details for SAML triggers.
#1 24785 nathan_fiedler Add SAML triggers.


I wrote this a couple ago and thought about it again today. I miss street witnessing. I miss being on an adventure with Jesus. I miss making a real difference, the internet is a good tool, but with so many demons trolling everywhere it sometimes makes me feel like nothing I say on here will ever make a difference to anyone.


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text:
Matt Kuchar is 2 shots behind Dustin Johnson a week after caddie debacle
Orlando Ramirez-USA TODAY Sports
By Steve DiMeglio February 22, 2019 8:20 pm Follow	@Steve_DiMeglio
By Steve DiMeglio | February 22, 2019 8:20 pm	Follow @Steve_DiMeglio
MEXICO CITY – Matt Kuchar's doing his best to change the narrative.
With four birdies to begin his second round Friday, Kuchar came home with a 4-under-par 67 that left him two shots out of the lead set by Dustin Johnson in the World Golf Championships-Mexico Championship at Club de Golf Chapultepec.
"I just want to keep playing consistent golf," Kuchar said. "I'm pleased with the state of my game at the moment."
It's a much better place for Kuchar to be than where he was last week in the Genesis Open at Riviera Country Club. He was in the middle of a caddie scandal that threatened his reputation, which up until then was spotless.
Instead of talking about golf, Kuchar, long a fan favorite, had to address his payment to David 'El Tucan' Ortiz, who was a fill-in caddie for Kuchar when he won the Mayakoba Golf Classic and its $1.3 million first prize last year.
Kuchar originally paid Ortiz $5,000 for his week's work – a deal the two agreed upon. But when news broke of the sum – which accounted for less than 0.4 percent of Kuchar's winnings, far below the standard 10 percent ($130,000) regular Tour caddies receive when their boss wins – Kuchar came under intense criticism.
At first, Kuchar defended his payment, which led to more criticism that he was out of touch, cheap and insensitive. Then he doubled down, and as some said on social media, he kept putting his own feet in his mouth. Fans at Riviera hurled biting remarks at Kuchar throughout his four rounds.
Upon reflection – he said he cringed when he read the words of his defense – Kuchar had a change of heart.
"Listen, I was stubborn, hard-headed," Kuchar said last week. "In my mind, I had it as 'a deal is a deal.' But after I won the tournament, a deal wasn't a deal. Any transaction, all parties should come out feeling like they've won, and certainly in David's case he did not feel like he won in that situation.
"I need to make it right. It's as simple as that."
Kuchar sent an additional $45,000 to Ortiz and made a charitable contribution to the Mayakoba Golf Classic.
In his first two rounds in the Mexico Championship, Kuchar hasn't heard one insult from anyone in the gallery. The familiar "Kooch," shouts were loud and clear. After the second round, Kuchar gladly spoke to the four birdies he made to start the round, his fondness for the tree-lined golf course, his success in driving the ball well.
What he really didn't want to do is rehash last week.
"I don't know if I would say that," Kuchar responded when asked if playing well this week was helping him put last week behind him. "I like to play well every week kind of regardless, but it is nice. It is nice to have a good showing, it is nice to kind of be back in the hunt again.
"Listen, golf is so much more fun when you have a chance to win, and it's been a lot of fun this week just playing some good golf. Having a chance with 36 holes to play is a good place to be."
Shackelford: Rise of 'backstopping' drives at integrity of golf
Rickie Fowler says new rule is terrible after he's handed one-shot penalty for illegal drop
Shot-By-Shot Recap: Tiger Woods (-5) goes low with 66 Friday at WGC-Mexico
Matt Kuchar, WGC Mexico, WGC-Mexico Championship 2019, PGA Tour, Professional


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text:
\section{Introduction}

The term dibaryon is used somewhat ambiguously in the literature.
It is applied for single hadrons viewed as genuine compact
six-quarks states that are tied together
by (rather short-ranged) gluon-exchange forces between the quarks, on
one hand side, but also for loosely bound two-baryons systems
such as the deuteron,
that are formed by long-ranged forces between their constituents.
Possibly the most famous one of the former kind
is the $H$-dibaryon which was predicted by Jaffe in
1977 as a deeply bound state with quantum numbers of the
$\Lambda\Lambda$ system, i.e. strangeness ${S}=-2$ and isospin $I=0$,
and with $J^P=0^+$ \cite{Jaffe:1976yi}.

In any case, the aforementioned deuteron (the neutron-proton bound state in
the $^3S_1$-$^3D_1$ channel) is so far the only known and unambiguously
established dibaryon. The interaction in the $^1S_0$ partial wave
of the neutron-proton ($np$) system is just not strong enough to
produce a bound state and only a virtual state is created.
Certainly, there is no shortage of new proposals of
dibaryon candidates in nucleon-nucleon scattering \cite{Adlarson}
as well as in the strangeness sector \cite{Gal10}.
In particular, the (approximate) SU(3) flavor symmetry of the strong
interaction suggests that bound states could exist also in other systems
formed by two octet baryons \cite{Miller}.
Indeed meson-exchange models like the Nijmegen baryon-baryon ($BB$)
interaction \cite{Stoks:1999bz}, derived under the assumption of (broken) SU(3)
symmetry, predict bound states for the $\Xi\Xi$ but also for the
$\Xi\Sigma$ and $\Xi\Lambda$ systems.
A $BB$ interaction derived in a rather different way, namely within the
framework of chiral effective field theory (EFT) \cite{Polinder06,Polinder07}
generates likewise bound states in the strangeness $S=-3$ and $S=-4$
sectors \cite{Hai10a}.

With regard to the $H$-dibaryon, many experimental searches were carried out
over the years, but so far no convincing signal was found \cite{Yoon}.
Recently, however, the $H$-dibaryon was put back on the agenda by lattice
QCD calculations performed by the NPLQCD \cite{Beane,Beane11a} and HAL QCD
\cite{Inoue,Inoue11a} Collaborations, where evidence for a bound state in
the pertinent $BB$ channel was found.
The NLPQCD Collaboration reported also evidence for a $\Xi^-\Xi^-$ bound
state \cite{Beane11a}.
Nevertheless, one has to keep in mind that most present-day lattice QCD calculations
are not performed at the physical masses of the involved particles. Thus, it
is an open question how the binding energies of the calculated states evolve when
those masses approach their physical values. Standard chiral extrapolations
\cite{Beane11,Shanahan11} might reach their
limits in case of dynamically generated bound states where there is a
delicate interplay between the interaction potential (that depends on the pion mass)
and the kinetic energy (that is affected by the baryon masses). Specifically
in situations where two or more $BB$ channels can couple, as it is the case for
the $H$-dibaryon, the effects due to the baryon masses could be sizeable.

In this paper, we analyze various issues related to lattice QCD calculations
in the framework of chiral effective field theory  for the $BB$
interaction at leading order (LO) in the Weinberg counting.
Indeed, the framework of chiral effective field theory in which our
$BB$ interactions are derived is very well suited to shed light
on the general characteristics of possible dibaryon bound states
and, in particular, to study the
quark mass\footnote{Because of the Gell-Mann-Oakes-Renner relation, the pion mass
squared is proportional to the average light quark mass. Therefore, the notions
``quark mass dependence'' and ``pion mass dependence'' can be used synonymously.}
dependence of the binding energies of those states,
in complete analogy to calculations of the quark mass dependence of the deuteron
binding energy performed in Refs.~\cite{Beane:2002vs,Beane03,Epe02,Epe02a}.
Another important issue that can be addressed here is how this quark mass
dependence is affected when the SU(3) breaking manifested in the masses
of the octet baryons is accounted for.

The imposed (approximate) SU(3) flavor symmetry fixes the interactions
in the $S=-3$ and $S=-4$ sectors uniquely, once the (five) low-energy
constant (LECs) that occur at LO in chiral EFT are determined
by a fit to the available hyperon-nucleon data.
In particular, our LO interaction published in \cite{Polinder06}
implies the existence of several bound states in those systems.
It will be interesting to see how the corresponding binding energies
evolve when we increase the pion mass in order to match with the
conditions of present lattice QCD calculations
\cite{Beane,Beane11a,Inoue,Inoue11a}.

In the $S=-2$ sector with isospin zero where the $H$-dibaryon is expected
there is one additional LEC, corresponding to the SU(3) flavor-singlet channel,
that can not be fixed by hyperon-nucleon data.
Since the scarce experimental information available for this sector
($\Xi^-p \to \Xi^-p$ and $\Xi^-p \to \Lambda\Lambda$
cross sections \cite{Ahn:2005jz}) is afflicted with large uncertainties and
does not allow to constrain its value \cite{Polinder07},
one can exploit this freedom and fine-tune the remaining LEC to produce a
bound $H$ with a given binding energy, and then study its properties
\cite{Haidenbauer11}.
The case of the $H$-dibaryon is also very well suited to examine
the effects from the SU(3) breaking in the baryon masses
because, as said before, for the quantum numbers in question there are three
baryon-baryon channels that can couple,
namely $\Lambda\Lambda$, $\Xi N$, and $\Sigma\Sigma$.
Their physical thresholds are well separated, whereas in a completely SU(3)
symmetric world all $BB$ thresholds are degenerate.
We will see that this has very definite dynamical consequences.

Our manuscript is organized as follows: In Sec.~\ref{sec:2}, we recall the
basic formalism of the $BB$ interaction in the framework of chiral EFT.
Sec.~\ref{sec:3} contains a detailed discussion of the quark
mass dependence of binding energies in the strangeness $S=-3$ and $S=-4$
sectors, where our chiral EFT interaction but also the meson-exchange potential
of the Nijmegen group predict bound states in several $BB$ channels.
In Sec.~\ref{sec:4} we discuss in detail the situation for
the $H$ dibaryon. Specifically, we examine the influence of the SU(3)
breaking through the various two-baryon thresholds and we try to
make direct contact to the results published by the NPLQCD and
HAL QCD Collaborations.
The paper ends with some concluding remarks.

\section{The baryon-baryon interaction to leading order}
\label{sec:2}

For details on the derivation of the chiral $BB$ potentials for the strangeness sector
at LO using the Weinberg power counting, we refer the reader to
Refs.~\cite{Polinder06,Polinder07,Haidenbauer07},
see also Refs.~\cite{Savage1,Korpa,Savage2}.
Here, we just briefly summarize the basic ingredients of the chiral EFT for $BB$ interactions.
\begin{table*}[t]
\renewcommand{\arraystretch}{1.2}
\centering
\begin{tabular}{|l|c|c|l|c|l|}
\hline
&Channel &Isospin &$C_{1S0}$ &Isospin &$C_{3S1}$\\
\hline
$S=0$&$NN\rightarrow NN$ &$1$ & $C^{27}$ &$0$ &$C^{10^*}$\\
\hline
$S=-1$&$\Lambda N \rightarrow \Lambda N$ &$\frac{1}{2}$ &$\frac{1}{10}\left(9C^{27}+C^{8_s}\right)$
&$\frac{1}{2}$ &$\frac{1}{2}\left(C^{8_a}+C^{10^*}\right)$\\
&$\Lambda N \rightarrow \Sigma N$ &$\frac{1}{2}$ &$\frac{3}{10}\left(-C^{27}+C^{8_s}\right)$
&$\frac{1}{2}$ &$\frac{1}{2}\left(-C^{8_a}+C^{10^*}\right)$\\
&$\Sigma N \rightarrow \Sigma N$ &$\frac{1}{2}$ &$\frac{1}{10}\left(C^{27}+9C^{8_s}\right)$
&$\frac{1}{2}$ &$\frac{1}{2}\left(C^{8_a}+C^{10^*}\right)$\\
&$\Sigma N \rightarrow \Sigma N$ &$\frac{3}{2}$ &$C^{27}$
&$\frac{3}{2}$ &$C^{10}$\\
\hline
$S=-2$&$\Lambda\Lambda \rightarrow \Lambda\Lambda$ &$0$ & $\frac{1}{40}\left(27C^{27}+8C^{8_s}+5C^{1}\right)$
  & & \\
&$\Lambda\Lambda \rightarrow \Xi N$ &$0$ &$\frac{-1}{40}\left(18C^{27}-8C^{8_s}-10\,C^{1}\right)$
  & & \\
&$\Lambda\Lambda \rightarrow \Sigma\Sigma$ &$0$ &$\frac{\sqrt{3}}{40}\left(-3C^{27}+8C^{8_s}-5C^{1}\right)$
  & & \\
&$\Xi N \rightarrow \Xi N$ &$0$ &$\frac{1}{40}\left(12C^{27}+8C^{8_s}+20\,C^{1}\right)$
  &$0$ &$C^{8_a}$\\
&$\Xi N \rightarrow \Sigma\Sigma$ &$0$ &$\frac{\sqrt{3}}{40}\left(2C^{27}+8C^{8_s}-10\,C^{1}\right)$
  &$1$ &$\frac{\sqrt{2}}{6}\left(C^{10}+C^{10^*}-2C^{8_a}\right)$\\
&$\Sigma\Sigma \rightarrow \Sigma\Sigma$ &$0$ &$\frac{1}{40}\left(C^{27}+24C^{8_s}+15C^{1}\right)$
 &$1$ &$\frac{1}{6}\left(C^{10}+C^{10^*}+4C^{8_a}\right)$\\
&$\Xi N \rightarrow \Xi N$ &$1$ &$\frac{1}{5}\left(2C^{27}+3C^{8_s}\right)$
  &$1$ &$\frac{1}{3}\left(C^{10}+C^{10^*}+C^{8_a}\right)$\\
&$\Xi N \rightarrow \Sigma\Lambda$ &$1$ &$\frac{\sqrt{6}}{5}\left(C^{27}-C^{8_s}\right)$
  &$1$ &$\frac{\sqrt{6}}{6}\left(C^{10}-C^{10^*}\right)$\\
&$\Sigma\Lambda \rightarrow \Sigma\Lambda$ &$1$ &$\frac{1}{5}\left(3C^{27}+2C^{8_s}\right)$
  &$1$ &$\frac{1}{2}\left(C^{10}+C^{10^*}\right)$\\
&$\Sigma\Lambda \rightarrow \Sigma\Sigma$ &   &   &$1$ &$\frac{\sqrt{3}}{6}\left(C^{10}-C^{10^*}\right)$\\
&$\Sigma\Sigma \rightarrow \Sigma\Sigma$ &$2$ &$C^{27}$
  & & \\
\hline
$S=-3$&$\Xi\Lambda \rightarrow \Xi\Lambda $ &$\frac{1}{2}$ &$\frac{1}{10}\left(9C^{27}+C^{8_s}\right)$
&$\frac{1}{2}$ &$\frac{1}{2}\left(C^{8_a}+C^{10}\right)$\\
&$\Xi \Lambda \rightarrow \Xi \Sigma $ &$\frac{1}{2}$ &$\frac{3}{10}\left(-C^{27}+C^{8_s}\right)$
&$\frac{1}{2}$ &$\frac{1}{2}\left(-C^{8_a}+C^{10}\right)$\\
&$\Xi \Sigma \rightarrow \Xi \Sigma $ &$\frac{1}{2}$ &$\frac{1}{10}\left(C^{27}+9C^{8_s}\right)$
&$\frac{1}{2}$ &$\frac{1}{2}\left(C^{8_a}+C^{10}\right)$\\
&$\Xi \Sigma \rightarrow \Xi \Sigma $ &$\frac{3}{2}$ &$C^{27}$
&$\frac{3}{2}$ &$C^{10^*}$\\
\hline
$S=-4$&$\Xi\Xi\rightarrow \Xi\Xi$ &$1$ & $C^{27}$ &$0$ &$C^{10}$\\
\hline
\end{tabular}
\caption{Various LO baryon-baryon contact potentials for the ${}^1S_0$ and ${}^3S_1$ partial
waves in the isospin basis. $C^{27}$ etc. refers to the corresponding ${\rm SU(3)_f}$
irreducible representation.}
\label{tab:1}
\end{table*}
\renewcommand{\arraystretch}{1.0}

The LO potential consists of four-baryon contact terms without derivatives and of
one-pseudoscalar-meson exchanges.
 The LO ${\rm SU(3)}_{\rm f}$ invariant contact terms for the octet $BB$
interactions that are Hermitian
and invariant under Lorentz transformations follow from the Lagrangians
\begin{eqnarray}
{\mathcal L}^1 &=& C^1_i \left<\bar{B}_a\bar{B}_b\left(\Gamma_i B\right)_b\left(\Gamma_i B\right)_a\right>\ , \quad
{\mathcal L}^2 = C^2_i \left<\bar{B}_a\left(\Gamma_i B\right)_a\bar{B}_b\left(\Gamma_i B\right)_b\right>\ , \nonumber \\
{\mathcal L}^3 &=& C^3_i \left<\bar{B}_a\left(\Gamma_i B\right)_a\right>\left<\bar{B}_b\left(\Gamma_i B\right)_b\right>\  .
\label{eq:2.1}
\end{eqnarray}
Here $a, b$ denote the Dirac indices of the particles, $B$ is the irreducible octet (matrix)
representation of ${\rm SU(3)}_{\rm f}$, and the $\Gamma_i$ are the usual elements of the
Clifford algebra \cite{Polinder06}. As described in Ref.~\cite{Polinder06},
to LO the Lagrangians in Eq.~(\ref{eq:2.1}) give rise to only six independent
low-energy constants (LECs), the $C_i^j$ in Eq.~(\ref{eq:2.1}), due to
${\rm SU(3)}_{\rm f}$ constraints. They need to be determined by a fit to experimental data.
It is convenient to re-express the $BB$ potentials in terms of the ${\rm SU(3)_f}$
irreducible representations, see e.g. Refs.~\cite{Swart,Dover}.
Then the contact interaction is given by
\begin{equation}
V=
\frac{1}{4}(1-\mbox{\boldmath $\sigma$}_1\cdot \mbox{\boldmath $\sigma$}_2) \, C_{1S0}
+ \frac{1}{4}(3+\mbox{\boldmath $\sigma$}_1 \cdot\mbox{\boldmath $\sigma$}_2) \, C_{3S1} \ ,
\label{contact}
\end{equation}
and the constraints imposed by the assumed ${\rm SU(3)}_{\rm f}$ symmetry on the interactions
in the various $BB$ channels for the $^1S_0$ and $^3S_1$ partial waves can be
readily read off from Table~\ref{tab:1}.

The lowest order ${\rm SU(3)}_{\rm f}$ invariant pseudoscalar-meson--baryon
interaction Lagrangian embodying the appropriate symmetries was also discussed in \cite{Polinder06}.
The invariance under ${\rm SU(3)}_{\rm f}$
transformations implies specific relations between the various coupling constants, namely
\begin{equation}
\begin{array}{rlrlrl}
f_{NN\pi}  = & f, & f_{NN\eta_8}  = & \frac{1}{\sqrt{3}}(4\alpha -1)f, & f_{\Lambda NK} = & -\frac{1}{\sqrt{3}}(1+2\alpha)f, \\
f_{\Xi\Xi\pi}  = & -(1-2\alpha)f, &  f_{\Xi\Xi\eta_8}  = & -\frac{1}{\sqrt{3}}(1+2\alpha )f, & f_{\Xi\Lambda K} = & \frac{1}{\sqrt{3}}(4\alpha-1)f, \\
f_{\Lambda\Sigma\pi}  = & \frac{2}{\sqrt{3}}(1-\alpha)f, & f_{\Sigma\Sigma\eta_8}  = & \frac{2}{\sqrt{3}}(1-\alpha )f, & f_{\Sigma NK} = & (1-2\alpha)f, \\
f_{\Sigma\Sigma\pi}  = & 2\alpha f, &  f_{\Lambda\Lambda\eta_8}  = & -\frac{2}{\sqrt{3}}(1-\alpha )f, & f_{\Xi\Sigma K} = & -f.
\end{array}
\label{su3}
\end{equation}
Here $f\equiv g_A/2F_\pi$, where $g_A$ is the nucleon axial-vector strength
and $F_\pi$ is the weak pion
decay constant.  We use the values $g_A= 1.26$ and $F_\pi = 92.4$~MeV.
For $\alpha$, the $F/(F+D)$-ratio \cite{Polinder06}, we adopt
the SU(6) value: $\alpha=0.4$, which is consistent with recent determinations
of the axial-vector coupling constants \cite{Ratcliffe,Yamanishi}.

The spin-space part of the LO one-pseudoscalar-meson-exchange potential is similar to the
static one-pion-exchange potential in chiral EFT for nucleon-nucleon
interactions, see e.g. \cite{Epe98} (recoil and relativistic corrections give
higher order contributions),
\begin{eqnarray}
V^{B_1B_2\to B_1'B_2'}&=&-f_{B_1B_1'P}f_{B_2B_2'P}\frac{\left(\mbox{\boldmath $\sigma$}_1\cdot{\bf q}\right)\left(\mbox{\boldmath $\sigma$}_2\cdot{\bf q}\right)}{{\bf q}^2+M^2_P}\ ,
\label{eq:14}
\end{eqnarray}
where $M_P$ is the mass of the exchanged pseudoscalar meson. The transferred
momentum ${\bf q}$ is defined in terms of the final and initial
center-of-mass (c.m.) momenta of the baryons, ${\bf p}'$ and ${\bf p}$, as
${\bf q}={\bf p}'-{\bf p}$.
In the calculation we use the (isospin averaged) physical masses of the exchanged
pseudoscalar mesons, i.e.
$M_\pi = 138.04\,$MeV, $M_K = 495.66\,$MeV, and $M_\eta = 548.8\,$MeV.
The explicit ${\rm SU(3)}$ breaking reflected in the mass splitting between the
pseudoscalar mesons and, in particular, the small mass of the pion relative to
the other members of the octet leads to sizeable differences in the range of
the interactions in the different channels and, thus, induces an essential dynamical
breaking of ${\rm SU(3)}$ symmetry in the $BB$ interactions.
The $\eta$ meson was identified with the octet $\eta$ ($\eta_8$) and its physical
mass was used. Note that for getting the actual potential for a specific channel
one still has to multiply the expression in Eq.~(\ref{eq:14}) with the pertinent
isospin coefficient (as given, e.g., in Ref.~\cite{Polinder06}).

The reaction amplitudes are obtained from the solution of a coupled-channel
Lippmann-Schwinger (LS) equation for the interaction potentials:
\begin{eqnarray}
&&T_{\rho''\rho'}^{\nu''\nu',J}(p'',p';\sqrt{s})=V_{\rho''\rho'}^{\nu''\nu',J}(p'',p')+
\sum_{\rho,\nu}\int_0^\infty \frac{dpp^2}{(2\pi)^3} \, V_{\rho''\rho}^{\nu''\nu,J}(p'',p)
\frac{2\mu_{\nu}}{q_{\nu}^2-p^2+i\eta}T_{\rho\rho'}^{\nu\nu',J}(p,p';\sqrt{s})\ .
\label{LS}
\end{eqnarray}
The label $\nu$ indicates the particle channels and the label $\rho$ the partial wave.
$\mu_\nu$ is the pertinent reduced mass. The on-shell momentum in the intermediate state,
$q_{\nu}$, is defined by $\sqrt{s}=\sqrt{m^2_{B_{1,\nu}}+q_{\nu}^2}+\sqrt{m^2_{B_{2,\nu}}+q_{\nu}^2}$.
Relativistic kinematics is used for relating the laboratory energy $T_{{\rm lab}}$ of the hyperons
to the c.m. momentum.

In \cite{Polinder06,Polinder07}
the LS equation was solved in the particle basis, in order to incorporate the correct physical
thresholds. Since here we are primarily interested in bound states we work in the isospin
basis. Furthermore, we ignore the Coulomb interaction (as it is also done in
the pertinent lattice QCD calculations).
We use the following (isospin averaged) baryon masses: $m_N=939.6$ MeV,
$m_{\Lambda}=1115.6$ MeV, $m_{\Sigma}=1192.5$ MeV, and $m_\Xi=1318.1$ MeV.
In the $S=-4$ and $S=-3$ sectors either single channel ($\Xi\Xi$) or
coupled-channel ($\Xi\Lambda - \Xi\Sigma$) equations have to be solved. For $S=-2$ and,
in particular, for the $H$-dibaryon there are three coupled channels, namely ${\Lambda}\La$, $\Xi N$
and ${\Sigma}\Si$. The potentials in the LS
equation are cut off with a regulator function, $\exp\left[-\left(p'^4+p^4\right)/\Lambda^4\right]$,
in order to remove high-energy components of the baryon and pseudoscalar meson fields \cite{Epe05}.
We consider cut-off values in the range from 550 to 700 MeV, similar to what was used for
chiral $NN$ potentials \cite{Epe05}.

The imposed ${\rm SU(3)}$ flavor symmetry implies that only five of the six LECs
contribute to the $YN$ interaction, namely $C^{27}$, $C^{10}$, $C^{10^*}$, $C^{8_s}$,
and $C^{8_a}$, cf. Table~\ref{tab:1}.
These five contact terms were determined in
\cite{Polinder06} by a fit to the $YN$ scattering data. Since the $NN$ data
cannot be described with a LO EFT (except very close to the threshold),
${\rm SU(3)}$ constraints from the $NN$ interaction
were not implemented explicitly. As shown in Ref.~\cite{Polinder06},  a good
description  of the 35 low-energy $YN$ scattering can be
obtained for cutoff values $\Lambda=550,...,700$ MeV and for natural values of the LECs.
The sixth LEC ($C^{1}$) is only present in the $S=-2$ channels with isospin zero,
cf. Table~\ref{tab:1}. There is scarce experimental information on these
channels that could be used to fix this LEC, but it turned out that the quality
of the existing data does not really allow to constrain its value reliably
\cite{Polinder07}. Even with the value of the sixth LEC chosen so that
$C^{{\Lambda}\La\to {\Lambda}\La}_{1S0} = 0$, agreement with those data can be achieved. In this case
a scattering length of $a_{^1S_0}^{\Lambda\Lambda} = -1.52$~fm \cite{Polinder07}
is obtained.
Analyses of the measured binding energy of the double-strange hypernucleus
${}^{\;\;\;6}_{\Lambda\Lambda}{\rm He}$ \cite{Takahashi:2001nm} suggest that
the ${\Lambda}\La$ scattering length could be in the range of
$-1.3$ to $-0.7$ fm \cite{Gal,Rijken,Fujiwara}.
A first determination of the scattering length utilizing data on the
$\Lambda\Lambda$ invariant mass from the reaction
$^{12}C(K^-,K^+\Lambda\Lambda X)$ led to the result
$a^{\Lambda\Lambda}=-1.2\pm 0.6$ fm \cite{Ashot}.

\section{Quark mass dependence of baryon-baryon binding energies}
\label{sec:3}

As discussed in Ref.~\cite{Hai10a}, our LO chiral EFT interaction
predicts several bound states for the strangeness $S=-3$ and $S=-4$
sectors.
Let us start with the ${}^1S_0$ partial wave in the $\Xi^0\Lambda$
channel. For the smallest cut-off ($\Lambda = 550$ MeV) only a virtual
state is found in this partial wave which, however,
eventually transforms into a real bound state when the cut-off is increased
within the considered range. For the largest cut-off (700 MeV) a binding
energy of $-0.43\,$MeV is predicted.
The results for the $\Xi^0\Lambda$ channel of other potentials that provide
detailed results for the $S=-3$ and $S=-4$ sectors \cite{Stoks:1999bz,Fujiwara}
suggest also an overall attractive interaction in the ${}^1S_0$ partial
wave though only a very moderate one which does not support a bound state.

The $S$-waves in the $\Xi\Sigma$ $I=3/2$ channel belong to the same
($10^*$ and $27$, respectively, cf. Table~\ref{tab:1})
irreducible representations where in the $NN$ case bound states
(${}^3S_1$-$^3D_1$) or virtual states (${}^1S_0$) exist.
Therefore, one expects that such states can also occur for $\Xi\Sigma$.
Indeed, here bound states are present for both partial waves in the Nijmegen
model, cf. the discussion in Sect.~III.B in Ref.~\cite{Stoks:1999bz}.
The chiral EFT interaction has a bound state too for ${}^1S_0$,
for all cut-off values \cite{Hai10a}. The binding energies lie in
the range of $-2.23\,$MeV ($\Lambda = 550\,$MeV) to $-6.15\,$MeV (700 MeV).
But in the ${}^3S_1$-$^3D_1$ partial wave the attraction is obviously not
strong enough to form a bound state.
The ${}^1S_0$ state of the $\Xi\Xi$ channel belongs also to the $27$plet
irreducible representation and also here the Nijmegen as well as the
chiral EFT interactions produce bound states. In our case the binding energy
lies in the range of $-2.56\,$MeV ($\Lambda = 550\,$MeV) to $-7.28\,$MeV
(700 MeV).

\begin{figure}[t!]
\centering
\includegraphics[width=0.305\textwidth,keepaspectratio,angle=-90]{mxx.ps}
\includegraphics[width=0.305\textwidth,keepaspectratio,angle=-90]{mxl.ps}
\includegraphics[width=0.305\textwidth,keepaspectratio,angle=-90]{mxs.ps}
\caption{Dependence of the binding energies in different $S=-3$ and $S=-4$ $^1S_0$ partial waves
on the pion mass.
}
\label{fig:BE1}
\end{figure}

Since the ${}^1S_0$ partial waves in the $\Sigma N$ ($I=3/2$) and
$\Sigma\Sigma$ ($I=2$) channels belong likewise to the $27$plet, cf.
Table~\ref{tab:1}, one could expect bound states in those states, too.
However, our chiral EFT interaction is only moderately attractive in the
former case, as reflected in the corresponding scattering lengths
which range from $-2.24$ to $-2.36\,$fm, cf. \cite{Polinder06}. There
is also no bound state for $\Sigma^+\Sigma^+$, though the predicted
scattering lengths are here between $-6.23$ to $-9.42\,$fm, which is an
indication that there is a virtual state not too far from the physical
region.
Note that in our calculation
$\Sigma \Sigma \,(I=2) \equiv \Sigma^+\Sigma^+ \equiv \Sigma^-\Sigma^-$
and, therefore, we use those designations synonymously here.
The Nijmegen NSC97 potential, on the other hand, clearly produces
a bound state in the $\Sigma^+\Sigma^+$ state, as signalled by the
large and positive scattering lengths \cite{Stoks:1999bz}.
Interestingly, a $BB$ interaction derived within the constituent quark-model
(fss2) \cite{Fujiwara}, yields also a scattering length that is very large
and negative so that there should be a virtual state practically at the
$\Sigma^+\Sigma^+$ threshold. On the other hand, for all $S=-3$ and $S=-4$
partial waves no bound states are predicted by this interaction model
based on quark-gluon dynamics \cite{Fujiwara}.

Let us now consider variations of the masses of the involved particles.
First we study the dependence of the binding energies on the pion
mass $M_\pi$ and keep the baryon masses at their physical values.
We will examine the specific situation for the concrete (meson and
baryon) masses that correspond to the calculation reported by the NPLQCD
Collaboration below.

Our results are displayed in Figs.~\ref{fig:BE1} and \ref{fig:BE2}.
Obviously for the $S=-3$ and $S=-4$ systems (Fig.~\ref{fig:BE1})
there is a fairly weak dependence of the predicted binding energies
on the pion mass. In particular, the variation from the physical point
to masses around 400 MeV, corresponding to the present status of
the NPLQCD computations, are relatively small compared to the differences
due to the cut-off variations.
Note that for $\Xi\Sigma$
the binding energy decreases with increasing pion mass, in contrast to
what happens in the other channels.

Results for the $S=-1$ and $S=-2$ systems are presented in Fig.~\ref{fig:BE2}.
Contrary to the $\Lambda\Lambda$ system, which we discuss in the
next section, the $\Sigma\Sigma$ interaction in the $I=2$ channel is
completely fixed by the five LECs that could be determined by
a fit to the $YN$ data, cf. Table~\ref{tab:1}. Thus predictions can be
made for this system too. Interestingly, while being unbound at the
physical point, a bound $\Sigma^+\Sigma^+$ state is created when the
pion mass is increased. For $M_\pi\approx$ 400 MeV the predicted
binding energy is around 2-3 MeV. Note that corresponding investigations
within lattice QCD remained inconclusive in this case \cite{Beane11a}.
A bound state appears too in the $\Sigma^+ p$ system, however, only for
pion masses above 400 MeV.
Note that $\Sigma N \, (I=3/2) \equiv \Sigma^+ p \equiv \Sigma^- n$.
For both systems we observe a somewhat stronger
dependence of the binding energies on the pion mass as compared to
$S=-3$ and $S=-4$.

The dependence on the pion mass can be easily understood, on a
qualitative level, by considering the contributions from
pseudoscalar-meson exchange to the interaction in the various
baryon-baryon systems.
Though in a fully SU(3) symmetric world
\begin{equation}
V^{NN\to NN}_{(I=1)} =  V^{\Sigma N\to \Sigma N}_{(I=3/2)} =
V^{\Sigma\Sigma \to \Sigma\Sigma}_{(I=2)} =
V^{\Xi\Sigma\to \Xi\Sigma}_{(I=3/2)} = V^{\Xi\Xi\to \Xi\Xi}_{(I=1)} = V^{27}
\end{equation}
in the $^1S_0$ partial wave,
one has to keep in mind that the indivudal contributions of the pseudoscalar
mesons differ for different channels. Their relative strengths in the various
channels follows from the product of the relevant coupling constants, fixed
by the assumed SU(3) symmetry, which are tabulated in Eq.~(\ref{su3}), and
a corresponding isospin factor:

\renewcommand{\arraystretch}{1.2}
\begin{equation}
\begin{array}{llll}
NN \to NN: \ \ & V_\pi \propto \phantom{(20/25) \times} f^2, & V_\eta \propto {(3/25)} \times f^2 & \\
\Sigma N \to \Sigma N: & V_\pi \propto {(20/25)} \times f^2, & V_\eta \propto {(6/25)} \times f^2,
& V_K \propto {(2/25)} \times f^2 \\
\Sigma\Sigma \to \Sigma\Sigma: & V_\pi \propto {(16/25)} \times f^2,
& V_\eta \propto {(12/25)} \times f^2 & \\
\Xi\Sigma \to \Xi\Sigma: & V_\pi \propto {(-4/25)} \times f^2, \ \ &
V_\eta \propto {(-18/25)} \times f^2, \ \ & V_K \propto 2 \times f^2 \\
\Xi\Xi \to \Xi\Xi: & V_\pi \propto {(1/25)} \times f^2, & V_\eta \propto {(27/25)} \times f^2 & \\
\end{array}
\label{coupling}
\end{equation}
\renewcommand{\arraystretch}{1.0}

Let us compare, for example, $NN$ and $\Xi\Xi$. Obviously in the $NN$ case
the pion-exchange contribution dominates while
for $\Xi\Xi$ practically the whole contribution from pseudoscalar-meson
exchange is due to the $\eta$ meson. Consequently, variations of the
pion mass (or the SU(3) breaking manifested by the small pion mass)
are much less important for the $\Xi\Xi$ system than for
the $NN$ interaction, cf. Refs.~\cite{Beane:2002vs,Beane03,Epe02,Epe02a}
for a discussion of the effects in the latter system.
Since the small value $f_{\Xi\Xi\pi}  = -0.2 \times f$ enters also into the
$\Xi\Sigma$ interaction a similarly weak dependence is seen there. Note that
$V^{\Xi\Sigma\to \Xi\Sigma }_\pi = - 4 \times V^{\Xi\Xi \to \Xi\Xi}_\pi$ for
the isospin channels shown in Fig.~\ref{fig:BE1}, which explains the opposite
trend in the dependence of the binding energy on the pion mass.
In case of $\Xi\Lambda$, pion-exchange contributes only via coupled-channel
effects so that one expects a weak pion-mass dependence anyway.
In the channels $\Sigma N$ and $\Sigma\Sigma$ where the strength of
pion exchange is less reduces as compared to $NN$
($V^{\Sigma N \to \Sigma N}_\pi = 4/5 \times V^{NN\to NN}_\pi$,
$V^{\Sigma \Sigma \to \Sigma \Sigma}_\pi = 16/25 \times V^{NN\to NN}_\pi$)
we observe a sizeable pion mass dependence of the binding energies, cf.
Fig.~\ref{fig:BE2}.
Similar comments also apply for the pion mass dependence of the
baryon octet states with increasing strangeness \cite{Frink:2005ru}.
Note that the relations in Eq.~(\ref{coupling}) follow for the SU(6)
value $\alpha = 0.4$, but they change only marginally for values of
$\alpha \approx 0.36 - 0.37$, as determined recently in analyses of
hyperon semi-leptonic decay data \cite{Ratcliffe,Yamanishi}.

\begin{figure}[t!]
\centering
\includegraphics[width=0.305\textwidth,keepaspectratio,angle=-90]{msn.ps}
\includegraphics[width=0.305\textwidth,keepaspectratio,angle=-90]{mss.ps}
\caption{Dependence of the binding energies in the
$\Sigma^+ p$ (left) and $\Sigma^+ \Sigma^+$ (right) $^1S_0$ partial waves
on the pion mass.
}
\label{fig:BE2}
\end{figure}

In order to connect as closely as possible to the results published by the
NPLQCD Collaboration \cite{Beane11b} we performed also calculations with
meson and baryon masses corresponding precisely to those in the lattice
QCD simulation. Specifically, we use $M_\pi = 389\,$MeV,
$M_K = 544\,$MeV, and $M_\eta = 587\,$MeV, and the
baryon masses $m_N=1151.3\,$MeV, $m_{\Lambda}=1241.9\,$MeV, $m_{\Sigma}=1280.3\,$MeV,
and $m_\Xi=1349.6\,$MeV, all taken from Ref.~\cite{Beane11b}.
Corresponding results are summarized in Table \ref{BELQCD} where we also
include the binding energies at the physical point and those where only the
pion mass was set to $M_\pi = 389\,$MeV. All values are given with two digits
behind the comma in order to facilitate an easy comparison of the relative
size of the various effects. The absolute uncertainty of our leading-order
calculation is, of course, best reflected in the cut-off dependence of the
results represented by the shaded bands in Figs.~\ref{fig:BE1} and
\ref{fig:BE2} and by the pertinent values in Table \ref{BELQCD}.

The results in Table \ref{BELQCD} make clear that there are sizeable effects
from the baryon masses (and of the heavy pseudoscalar mesons $K$ and $\eta$,
too) on the binding energies. Specifically in the $S=-3$ and $S=-4$ sectors
those are more significant than the variations in the pion mass that we
considered, which is not surprising if one recalls the discussion above.
Clearly, one has to acknowledge that the systematic uncertainty in
the current lattice QCD calculations is still significantly larger
than those mass effects \cite{Beane11a}.
Despite of this, it is remarkable that the $\Xi^-\Xi^-$ binding
energy published in \cite{Beane11a}, $E_B = (-14.0 \pm 1.4 \pm 6.7)\,$MeV,
is rather well in line with the corresponding predictions based on LO chiral
EFT. Considering the (rather modest) mass dependence found in our calculation
we would expect that this state is still bound at the physical point,
namely by roughly 10 MeV if one takes the central value from \cite{Beane11a}
as guideline.
Future lattice QCD calculations with improved statistics will certainly resolve
this exciting issue, once the systematic uncertainties can be reduced.

With regard to the other states listed in Table~\ref{BELQCD} only the one
in the $\Xi^-\Sigma^-$ $^1S_0$ partial wave is likely to survive for
physical masses. All other states are fairly loosely bound already for masses
corresponding to the NPLQCD calculation and disappear when we go to the
physical point.

\begin{table}[h]
\renewcommand{\arraystretch}{1.5}
\centering
\begin{tabular}{|c|c|c|c|c|}
\hline
& \multicolumn{3}{|c|} {$\chi$EFT} & NPLQCD \cite{Beane11a} \\
\hline
                  & physical masses & $M_\pi = 389$ MeV & NPLQCD masses & \\
${\Lambda}$ [MeV] & 550 {$\cdot\cdot\cdot$} 700 & 550 {$\cdot\cdot\cdot$} 700 & 550 {$\cdot\cdot\cdot$} 700 & \\
\hline
\ $\Xi^-\Xi^- $         \ & \ $-2.56$ {$\cdot\cdot\cdot$} $-7.27$ \ & \ $-2.87$ {$\cdot\cdot\cdot$} $-7.93$ \ & \ $-3.92$ {$\cdot\cdot\cdot$} $-10.41$ \ &
 \ -14.0 $\pm$ 1.4 $\pm$ 6.7 \ \\
\ $\Xi^-\Lambda $       \ & \ $ \phantom{00}0 $ {$\cdot\cdot\cdot$} $-0.40$ \ & \ $ \phantom{00}0 $ {$\cdot\cdot\cdot$} $-1.26$ \
& \ $-1.05$ {$\cdot\cdot\cdot$} $-4.86$ \ & \\
\ $\Xi^-\Sigma^- $      \ & \ $-2.23$ {$\cdot\cdot\cdot$} $-6.18$ \ & \ $-1.25$ {$\cdot\cdot\cdot$} $-4.02$ \ & \ $-2.89$ {$\cdot\cdot\cdot$} $-7.93$ \
& \\
\ $\Sigma^-\Sigma^- $ \ & \ $ -  $ \ & \ $-0.42$ {$\cdot\cdot\cdot$} $-1.99$ \ & \ $-1.23$ {$\cdot\cdot\cdot$} $-3.93$ \
& inconclusive \\
\ $\Sigma^- n $       \ & \ $ -  $ \ & \ $ \phantom{00}0 \ ${$\cdot\cdot\cdot$} $-0.11$ \ & \ $-0.30$ {$\cdot\cdot\cdot$} $-1.56$ \
& \\
\hline
\end{tabular}
\caption{Binding energies in MeV of various $BB$ bound states in the $^1S_0$ partial wave
as obtained from the EFT potential for physical masses
(second column), for a pion mass of $M_\pi = 389$ MeV (third column),
and using meson and baryon masses that correspond to the lattice QCD calculation
of \cite{Beane11a} (fourth column). The last column are results of the lattice
QCD calculation taken from Ref.~\cite{Beane11a}.
}
\label{BELQCD}
\end{table}

In this context let us emphasize that, of course, it would be also interesting to
confirm or exclude the existence of those bound states experimentally.
The possibility to find signals for strange di-baryon states in heavy-ion collisions
was discussed in Refs.~\cite{Schaffner1999,Steinheimer}.
Also the new facilities J-PARC (Tokai, Japan) and FAIR (Darmstadt, Germany)
could allow one to obtain empirical constraints on the baryon-baryon interaction
in the $S=-3$ and $-4$ sector. Information could come from formation experiments
of corresponding hypernuclei or from proton-proton and antiproton-proton collisions
at such high energies that pairs of baryons with strangeness $S=-3$ or $S=-4$ can
be produced.

\section{The $H$-dibaryon}
\label{sec:4}

\subsection{General considerations}
As already said, in the $S=-2$ sector with isospin zero where the $H$-dibaryon
is expected there is one additional contact term (${C^1}$, cf. Table~\ref{tab:1}),
corresponding to the SU(3) flavor-singlet channel, that is not fixed by
hyperon-nucleon data and, therefore, no immediate predictions can be made.
In principle, this LEC could be determined from experimental information available
for this sector, but the scarce data
($\Xi^-p \to \Xi^-p$ and $\Xi^-p \to \Lambda\Lambda$
cross sections \cite{Ahn:2005jz}) are afflicted with large uncertainties
and do not allow to constrain its value \cite{Polinder07}.
Thus, in practice one can exploit this freedom and fine-tune the remaining
LEC to produce a bound $H$ with a given binding energy, and then study its
properties \cite{Haidenbauer11}. Indeed, it turned out that a near-threshold
bound state can be easily produced for ${C^1}$ values that are of natural size.

In the following we assume that the $H$-dibaryon is a (loosely) bound $BB$ state
\cite{Haidenbauer11}, just like the bound states discussed in the previous section.
We do not
consider the case where the $H$-dibaryon is a genuine 6-quark state as originally
suggested by Jaffe \cite{Jaffe:1976yi}. In fact, we cannot say anything about
the latter situation within our framework.
We also assume that the binding energy, $E_H$, is similar to
that of the deuteron ($D$) because this allows us to compare the properties
of the generated $H$-dibaryon directly with the familiar deuteron case.
Specifically, we fix the value of the flavor-singlet LEC ${C^1}$ in such a way that
the binding momentum is $\gamma_{H} = \gamma_{D} = 0.23161\,$fm
($E = - \gamma^2 / m_{B}$, where $m_{B}$ is either $m_N$ or $m_\Lambda$),
in view of the well-known relation between the binding energy and the effective
range parameters \cite{Schwinger47,Bethe}
\begin{equation}
\frac{1}{a} \simeq {\gamma} - \frac{1}{2}{r} {\gamma}^2 .
\nonumber
\end{equation}
This relation is very well fulfilled for the deuteron and the corresponding
neutron-proton $^3S_1$ scattering length ($a=5.43\,$fm) and effective range
($r=1.76\,$fm). One would naively expect that the same should happen for the
$H$-dibaryon. However, it turns out that the corresponding results for
${\Lambda}\La$ in the $^1S_0$ partial wave are quite different, namely
$a=3.00\,$fm and $r=-4.95\,$fm. Specifically, the effective range
is much larger and, moreover, negative. Clearly, the
properties of the $H$-dibaryon are not comparable to those of the
deuteron, despite the fact that both bound states are close to the
elastic threshold.
Indeed, if one recalls the expressions for the relevant potentials
as given in Table \ref{tab:1},
\begin{equation}
V^{{\Lambda}\La \rightarrow {\Lambda}\La} = \frac{1}{40}\left(27C^{27}+8C^{8_s}+{ 5}{
    C^{1}}\right) \, , \ \ \
V^{\Xi N \rightarrow \Xi N} = \frac{1}{40}\left(12C^{27}+8C^{8_s}+{ 20}{
    C^{1}}\right) \, ,
\nonumber
\end{equation}
one can see that the attraction provided by the SU(3) flavor-singlet state (i.e. $C^{1}$)
contributes with a much larger weight to the $\Xi N$ channel than to ${\Lambda}\La$.
This indicates that the presumed $H$-dibaryon could be predominantly a
$\Xi N$ bound state. We have confirmed this conjecture by evaluating explicitly
the phase shifts in the ${\Lambda}\La$ and $\Xi N$ channels, cf. the discussion in the
next section. Indeed, one finds that the phase shift for the $\Xi N$ channel
is rather similar to the $NN$ $^3S_1$ case. Specifically, the $\Xi N$ ($^1S_0$) phase shift
$\delta(q_{\Xi N})$ fulfills $\delta(0)-\delta(\infty) = 180^\circ$ in
agreement with the Levinson theorem.
The ${\Lambda}\La$ ($^1S_0$) phase behaves rather differently and
satisfies $\delta(q_{{\Lambda}\La}=0) - \delta(\infty) = 0$.
Note that there have been earlier discussions on this issue in
the context of $S=-2$ baryon-baryon interactions derived within the
quark model \cite{Oka,Nakamoto}.

The results above were obtained with the LECs $C^{27}$ and $C^{8_s}$
fixed from the $YN$ data for the cutoff value $\Lambda = 550$~MeV \cite{Polinder06}.
We considered also the other variants corresponding to cutoff masses
of 600, 650, and 700 MeV in the LS equation~(\ref{LS}), as in
Ref.~\cite{Polinder07}. But since the contact term $C^{1}$ has to be
determined anew in each case it turned out that the results are rather
similar for all cutoffs once $C^{1}$ is fixed in such a way that
the same binding energy for the $H$ dibaryon is produced. Thus,
we will present only results for the $\Lambda = 550$~MeV case.
We denote the $YY$ interaction with a loosely bound $H$ dibaryon by
YY-D in the following, and use the notation YY(550) for the
original interaction from Ref.~\cite{Polinder07}.

Let us now consider variations of the masses of the involved particles.
The dependence of the $H$ binding energy on the pion mass $M_\pi$ is
displayed in Fig.~\ref{fig:mpi} (left). For the YY-D potential considered
above, enlarging the pion mass to around 400 MeV
(i.e. to values in an order that corresponds to the NPLQCD calculation \cite{Beane})
increases the
binding energy to around 8 MeV and a further change of $M_\pi$ to 700 MeV
(corresponding roughly to the HAL QCD calculation \cite{Inoue}) yields then 13 MeV,
cf. the solid line.
Readjusting $C^1$ so that we predict a $H$ binding energy of 13.2 MeV for
$M_\pi=389$ MeV, corresponding to the latest result published by
NPLQCD~\cite{Beane11a}, yields the dashed curve.
It is obvious that the dependence on $M_\pi$ we obtain agrees -- at least
on a qualitative level -- with that presented in Ref.~\cite{Beane11}.
Specifically, our calculation exhibits the same trend (a decrease of the binding
energy with decreasing pion mass) and our binding energy of 9 MeV at the physical
pion mass is within the error bars of the results given in~\cite{Beane11}.
On the other hand, we clearly observe a non-linear dependence of the binding
energy on the pion mass. As a consequence, scaling our results to the binding
energy reported by the HAL QCD Collaboration \cite{Inoue} (30-40 MeV for
$M_\pi \approx 700-1000$~MeV) yields binding energies of more than 20 MeV
at the physical point, which is certainly outside of the range suggested in
Ref.~\cite{Beane11}. However, we note that for such large pion masses the LO
chiral EFT can not be trusted quantitatively.
We remark that in our simulations the curves corresponding to different binding
energies remained roughly parallel even up to such large values as suggested
by the HAL QCD Collaboration.

\begin{figure}[t!]
\centering
\includegraphics[width=0.305\textwidth,keepaspectratio,angle=-90]{mpi.ps}
\includegraphics[width=0.305\textwidth,keepaspectratio,angle=-90]{msi.ps}
\caption{Dependence of the binding energy of the $H$-dibaryon on the pion mass
$M_\pi$ (left) and on the $\Sigma$ mass $m_\Sigma$ (right).
The solid curve correspond to the case where $C^1$ is fixed such that $E_H = -1.87\,$MeV
for physical masses while for the dashed curve $C^1$ is fixed to yield $E_H = -13.2\,$MeV for
$M_\pi = 389$ MeV.
The asterisks and crosses represent results where, besides the
variation of $m_\Sigma$, $m_\Xi+m_N = 2 m_{\Lambda}$ is assumed so that the $\Xi N$ threshold
coincides with that of the ${\Lambda}\La$ channel.
The vertical (dotted) lines indicate the physical ${\Lambda}\La$ and ${\Sigma}\Si$ thresholds.
}
\label{fig:mpi}
\end{figure}

Our finding that any $H$-dibaryon is very likely a bound $\Xi N$ state rather than a ${\Lambda}\La$
state, which follows from the assumed (approximate) SU(3) symmetry of the interaction,
suggests that not only the pion mass but also the masses of the baryons play a significant
role for the concrete value of binding energy.
In the specific case of $J=0$, $I=0$, $S=-2$ we are dealing with three coupled channels,
namely ${\Lambda}\La$, $\Xi N$, and ${\Sigma}\Si$. For the isospin-averaged masses that we use
their thresholds are at 2231.2, 2257.7, and 2385.0~MeV, respectively.
Thus, the physical difference between the ${\Lambda}\La$ and $\Xi N$ thresholds of around
26~MeV implies that the $H$-dibaryon considered above is, in reality, bound by roughly
28~MeV with respect to its ``proper'' threshold. Accordingly, one intuitively expects that
in a fully SU(3) symmetric case, where the masses of all octet baryons coincide, the
bound state would remain more or less fixed to the $\Xi N$ threshold and then would lie also
about 28 MeV below the ${\Lambda}\La$ threshold.
Since we know from our experience with coupled-channel problems
\cite{Polinder06,Hai10a,Hai05,Hai11} that coupling effects are sizeable and
the actual separation of the various thresholds plays a crucial role we investigated also
the dependence of the $H$ binding energy on the thresholds (i.e. on the $\Sigma$, and on
the $\Xi$ and $N$ masses). Corresponding results are displayed in Fig.~\ref{fig:mpi} in
the right panel.

We start with considering the effect of the $\Sigma \Sigma$ channel because its threshold
is separated by roughly 154 MeV from the one of ${\Lambda}\La$ so that there is a rather
drastic breaking of the SU(3) symmetry. Indeed,
when we decrease the $\Sigma$ mass so that the nominal $\Sigma \Sigma$ threshold
(at 2385~MeV) moves downwards and finally coincides with the one of the
${\Lambda}\La$ channel (2231.2~MeV), we observe a concurrent fairly drastic
increase in the $H$ binding energy, cf. the solid curve in Fig.~\ref{fig:mpi} for
results based on the interaction YY-D with a binding energy of -1.87~MeV for
physical masses of the mesons and baryons.
In this context we want to point out that the direct
interaction in the $\Sigma\Sigma$ channel is actually repulsive for the low-energy
coefficients $C^{27}$ and $C^{8_s}$ fixed from the $YN$ data plus the pseudoscalar
meson exchange contributions with coupling constants determined from the SU(3)
relations Eq.~(\ref{su3}), and it remains repulsive even for $C^{1}$ values that produce
a bound $H$-dibaryon. But the coupling between the channels generates a sizeable
effective attraction which increases when the channel thresholds come closer.
The dashed curve is a calculation with the contact term $C^{1}$ fixed to simulate
the binding energy ($-13.2$~MeV) of the NPLQCD Collaboration at $M_\pi=389\,$MeV.
As one can see, the dependence of the binding energy on the $\Sigma$ mass is rather
similar. The curve is simply shifted downwards by around 4.5~MeV, i.e. by the difference
in the binding energy observed already at the physical masses.
The asterisks and crosses represent results where, besides the variation of the
$\Sigma\Sigma$ threshold, the $\Xi N$ threshold is shifted to coincide with that
of the ${\Lambda}\La$ channel. This produces an additional increase of the $H$ binding
energy by 20~MeV at the physical $\Sigma\Sigma$ threshold and by 9~MeV
for that case where all three $BB$ threshold coincide.
Altogether there is an increase in the binding energy of roughly 60~MeV
when going from the physical point to the case of baryons with identical
masses. This is significantly larger than the variations due to the pion mass
considered before. Note that we have kept the pion mass at its physical value
while varying the $BB$ thresholds.

\subsection{Comparison with lattice QCD results}

After these exemplary studies let us now try to connect with the published
$H$ binding energies from the lattice QCD calculations \cite{Beane11a,Inoue}.
The results obtained by the HAL QCD Collaboration are obviously for the SU(3)
symmetric case and the corresponding masses are given in Table I of
Ref.~\cite{Inoue}. Thus, we can take those masses and then fix the LEC
$C^1$ so that we reproduce their $H$ binding energy with those masses.
To be concrete: we use $M_{ps} = 673\,$MeV and $m_{B} = 1485\,$MeV, and fix
$C^1$ so that $E_H = -35\,$MeV. We denote this interaction by YY-HAL.
When we now let the masses of the baryons and
mesons go to their physical values the bound state moves up to the
${\Lambda}\La$ threshold, crosses the threshold, crosses also the $\Xi N$ threshold and
then disappears. In fact, qualitatively this outcome
can be already read off from the curves in Fig.~\ref{fig:mpi} by combining the
effects from the variations in the pion and the baryon masses. Based on those
results one expects a shift of the $H$ binding energy in the order of
60 to 70~MeV for the mass parameters of the HAL QCD calculation.

In case of the NPLQCD calculation we take the values provided in
Ref.~\cite{Beane11b}, as before. Those yield
then 17~MeV for the $\Xi N$-${\Lambda}\La$ threshold separation
(to be compared with the physical value of roughly 26~MeV) and
77~MeV for the ${\Sigma}\Si$-${\Lambda}\La$ separation (physical value around 154~MeV).
We also use the meson masses of Ref.~\cite{Beane11b}, specifically
$M_\pi = 389$ MeV.
With those baryon and meson masses we fix again the LEC $C^1$ so that we
reproduce the $H$ binding energy given by the NPLQCD Collaboration, namely
$E_H =-13.2$~MeV \cite{Beane11a} (called YY-NPL in the following).
Again we let the masses of the baryons and mesons approach their
physical values. Also here the bound state moves up to and crosses
the ${\Lambda}\La$ threshold. However, in the NPLQCD case the state survives
and remains below the $\Xi N$ threshold at the physical point. Specifically,
we observe a resonance at a kinetic energy of 21~MeV in the ${\Lambda}\La$
system or, more precisely, a quasi-bound state in the $\Xi N$ system around
5~MeV below its threshold.

\begin{figure}[t!]
\centering
\includegraphics[width=0.305\textwidth,keepaspectratio,angle=-90]{phla.ps}
\includegraphics[width=0.305\textwidth,keepaspectratio,angle=-90]{phxi.ps}
\includegraphics[width=0.305\textwidth,keepaspectratio,angle=-90]{phsi.ps}
\caption{Phase shifts in the $^1S_0$ partial wave in the $I=0$ channel of ${\Lambda}\La$ (a),
$\Xi N$ (b) and ${\Sigma}\Si$ (c) as a function of the pertinent laboratory energies.
The solid line is the result for our illustrative $BB$ interaction that produces a bound $H$ at
$E_H=-1.87\,$MeV.
The dotted line corresponds to the EFT potential of Ref.~\cite{Polinder07}
(Table 4) with cutoff mass $\Lambda = 550$ MeV.
The other curves are results for interactions that are fine-tuned to the
$H$ binding energies found in the lattice QCD calculations of the HAL QCD (dashed) and
NPLQCD (dash-dotted) Collaborations, respectively, for the pertinent meson (pion) and
baryon masses as described in the text.
}
\label{fig:phases}
\end{figure}

It is interesting to observe that the chiral extrapolation of the lattice
QCD results performed by Shanahan et al. \cite{Shanahan11} yields results
that are qualitatively similar to ours. In that reference the authors conclude
that the $H$-dibaryon is likely to be unbound by 13$\pm$14 MeV at the physical point.
Let us emphasize, however, that our values are not really comparable
with theirs. As said above, in our analysis we assume that the $H$-dibaryon is actually
a bound $BB$ state -- which seems to be the case also in the lattice QCD
studies \cite{Beane11a,Inoue}. On the other hand, in Ref.~\cite{Shanahan11} it is
assumed that the $H$ is a compact, multi-quark state rather than a loosely bound
molecular state, i.e. an object as originally suggested by Jaffe.
How such a genuine multi-quark state would be influenced
by variations of the $BB$ thresholds is completely unclear. It depends,
among other things, on whether and how strongly this state couples to the
${\Lambda}\La$, $\Xi N$, and ${\Sigma}\Si$ channels. So far there is no information
on this issue from lattice QCD calculations. Clearly, in case of a strong and
predominant coupling to the ${\Lambda}\La$ alone, variations of the ${\Sigma}\Si$ and
$\Xi N$ would not influence the $H$ binding energy significantly. However,
should it couple primarily to the $\Xi N$ and/or ${\Sigma}\Si$ channels
then we expect a sensitivity of the binding energy to their thresholds values
comparable to what we found in our study for the case of a bound state.

Phase shifts for the $^1S_0$ partial wave of the ${\Lambda}\La$, $\Xi N$ and
$\Sigma\Sigma$ channels are presented in Fig.~\ref{fig:phases}.
The solid line is the result for the $BB$
interaction YY-D that produces a loosely bound $H$ dibaryon with $E_H=-1.87$~MeV.
The phase shift for the $\Xi N$ channel, Fig.~\ref{fig:phases} (b), is rather similar to the
one for the $^3S_1$ $NN$ partial wave where the deuteron resides,
see e.g. \cite{Epe05}.
Specifically, it starts at $180^o$, decreases smoothly and eventually
approaches zero for large energies, fulfilling the Levinson theorem.
The result for ${\Lambda}\La$ ($^1S_0$), Fig.~\ref{fig:phases} (a), behaves rather differently.
This phase commences at zero degrees, is first negative but becomes positive within
20 MeV and finally turns to zero again for large energies.
The dashed curve corresponds to the interaction YY-HAL that was fitted to the
result of the HAL QCD Collaboration and reproduces their bound $H$ dibaryon with
their meson and baryon masses.
The phase shift of the $\Xi N$ channel, calculated with physical masses,
shows no trace of a bound state anymore. Still the phase shift
rises up to around $60^o$ near threshold, a behavior quite similar to that of
the $^1S_0$ $NN$ partial wave where there is a virtual state (also called
antibound state \cite{Kok,Pearce}). Indeed, such a virtual state also seems to
be present in the $\Xi N$ channel as a remnant of the original bound state.
The effect of this virtual state can be seen in the ${\Lambda}\La$ phase shift where it
leads to an impressive cusp at the opening of the $\Xi N$ channel,
cf. the dashed line in Fig.~\ref{fig:phases} (a).

In the $\Xi N$ phase shifts for the NPLQCD case (dash-dotted curve)
the presence of a bound state is clearly visible. The corresponding ${\Lambda}\La$
phase shift exhibits a resonance-like behavior at the energy where the
(quasi-bound) $H$ dibaryon is located.

The dotted curves are the results for the original chiral EFT potential
with cut-off $\Lambda = 550$ MeV as published in \cite{Polinder07}. The
${\Lambda}\La$ as well as the $\Xi N$ phase shifts are qualitatively similar
to the ones for the HAL QCD case. But the smaller $\Xi N$ phase shift
together with the reduced cusp effect indicate that there is no
near-by virtual state produced by this interaction.

The $\Sigma\Sigma$ phase shifts predicted by the various interactions are
almost the same, cf. Fig.~\ref{fig:phases} (c). This may be not too surprising.
After all, the
$\Sigma\Sigma$ threshold is rather far away from the one of the
$\Lambda\Lambda$ channel and the region, where we have introduced the $H$
dibaryon. Thus, it remains practically unaffected by those changes.

Finally, for illustrative purposes, we present cross sections for the
${\Lambda}\La$ and $\Xi^- p$ channels. Results of corresponding calculations,
now performed in particle basis (but neglecting the Coulomb interaction),
are displayed in Fig.~\ref{fig:cross}. There are some experimental constraints
for these two channels. In particular, there is an upper limit of $24$ mb at $90\%$
confidence level for elastic $\Xi^-p$ scattering,
while for the $\Xi^-p\rightarrow \Lambda\Lambda$ cross section at $p_{\rm lab}=500$ MeV/c
a value of $4.3^{+6.3}_{-2.7}$ mb was reported \cite{Ahn:2005jz}.

\begin{figure}[t!]
\centering
\includegraphics[width=0.305\textwidth,keepaspectratio,angle=-90]{crll.ps}
\includegraphics[width=0.305\textwidth,keepaspectratio,angle=-90]{crxmp.ps}
\includegraphics[width=0.305\textwidth,keepaspectratio,angle=-90]{crxmpll.ps}
\caption{Total cross sections for some $S=-2$ channels as a function of $p_{lab}$.
The solid line is the result for our illustrative $BB$ interaction that produces a bound $H$ at
$E_H=-1.87$ MeV. The dotted line corresponds to the EFT potential of Ref.~\cite{Polinder07}
(Table 4) with cutoff mass $\Lambda = 550$ MeV.
The other curves are results for interactions that are fine-tuned to the
$H$ binding energies found in the lattice QCD calculations of the HAL QCD (dashed) and
NPLQCD (dash-dotted) Collaborations, respectively, for the pertinent meson (pion) and
baryon masses as described in the text.
The experimental cross sections in (b) and (c) are taken from Ref. \cite{Ahn:2005jz}.
}
\label{fig:cross}
\end{figure}

As obvious from Fig.~\ref{fig:cross}, there are significant differences in the
cross sections predicted by the $YY$ interactions generated in the context of
the $H$-dibaryon discussion -- however, only at low momenta where no
experimental information is at hand so far. Anyhow, those results suggest that
a determination of the $\Xi^- p$ cross section at $p_{\rm lab} \approx 200$ MeV/c,
say, with reasonable errors would already put strong constraints on the
$H$-dibaryon. In particular, situations where it is located close to the $\Xi N$
threshold -- as at is the case in our simulations of the NPLQCD and HAL QCD results
(dash-dotted and dashed curves, respectively) -- could be ruled out.
Distinguishing an actually (though loosely) bound $H$-dibaryon (solid curve) from
the situation without any $H$-dibaryon (dotted curve) certainly requires better
statistics. Here one has to keep in mind that the $\Xi^-p$ cross section would
be even closer to the latter result, should the $H$-dibaryon be somewhat
stronger bound than assumed in our calculation. Note that the peak in the
$\Xi^- p$ cross section around 575 MeV/c is a cusp due to the opening of the
$\Sigma^0\Lambda$ channel.

There are also characteristic differences in the predictions for
$\Xi^- p\rightarrow \Lambda\Lambda$, cf. Fig.~\ref{fig:cross} (c).
However, since this cross section rises to infinity with decreasing $p_{\rm lab}$,
due to the phase-space factor, it might be more difficult to draw conclusions
in this case.

The assumed $H$ dibaryon below the ${\Lambda}\La$ threshold introduces a rather
strong and peculiar energy variation in the near-threshold ${\Lambda}\La$ cross
section, cf. the solid curve in Fig.~\ref{fig:cross} (a).
The effects due to the other considered interactions
is less spectacular, specifically, because the structure produced by the NPLQCD
case is so narrow that it would be presumably completely washed out once one
takes into account the finite momentum resolution of an actual experiment.
In any case, measuring the ${\Lambda}\La$ cross section directly seems to be
practically impossible. However, one could measure the ${\Lambda}\La$ invariant mass
spectrum in reactions like $K^- A \to {\Lambda}\La + X$ where $A$ can be the deuteron
or a heavier nucleus. As a matter of facts, corresponding results from a measurement
of $K^-\phantom{}^{12}\rm C$ have been already published \cite{Yoon}.
Still, it is unclear whether such an invariant mass distribution would
be dominated by the ${\Lambda}\La \to {\Lambda}\La$ transition amplitude or rather by
$\Xi N \to {\Lambda}\La$. Since our investigation suggests that any near-threshold
$H$-dibaryon will have a large if not dominant $\Xi N$ component
one expects that then the $\Xi N \to {\Lambda}\La$ amplitude should play
likewise an important if not decisive role for the ${\Lambda}\La$
invariant mass distribution.

\section{Summary}

In this paper we have presented an analysis of the quark mass dependence of
binding energies for baryon-baryon systems in the strangeness $S=-2$,
$S=-3$, and $S=-4$ sectors in the framework of chiral effective field
theory at leading order in the Weinberg counting.
In particular, we have explored the dependence of those binding energies
on the pion mass in order to connect with current lattice QCD calculations.
We remark that at higher orders, other effects like the quark mass dependence of
the meson-baryon couplings or of the contact interactions will have to be
considered (see e.g.~\cite{Epe02}).

With regard to the $\Xi\Xi$, $\Xi\Sigma$ and $\Xi\Lambda$ systems, where
meson-exchange potentials as well as leading-order EFT interactions,
derived under the assumption of (broken) SU(3) symmetry, predict
the existence of bound states in the various $^1S_0$ partial waves, we
find a rather weak dependence of the binding energies on the pion mass.
For the $\Xi^-\Xi^-$ system a calculation performed with meson and
baryon masses that match the status of a recent lattice QCD exploration
by the NPLQCD Collaboration yields binding energies that are
compatible with the reported lattice QCD result \cite{Beane11a}
within the given error bars.

We have also investigated the situation concerning the so-called $H$-dibaryon.
Here we found rather drastic effects caused by the SU(3) breaking related
to the values of the three thresholds $\Lambda\Lambda$, $\Sigma\Sigma$ and $\Xi N$.
For physical values the binding energy of the $H$ is reduced by as much as 60~MeV
as compared to a calculation based on degenerate (i.e. SU(3) symmetric) $BB$
thresholds.
Translating this observation to the situation in the HAL QCD \cite{Inoue}
calculation, we see that the bound state has disappeared at the physical point.
For the case of the NPLQCD calculation \cite{Beane11a},
a resonance in the $\Lambda\Lambda$ system might survive.

\ack
J.H. acknowledges stimulating discussions with N.N. Nikolaev.
This work is supported by the EU-Research
Infrastructure Integrating Activity ``Study of Strongly Interacting Matter''
(HadronPhysics2, grant n. 227431) under the Seventh Framework Program of the EU,
and by the DFG (SFB/TR 16 ``Subnuclear Structure of Matter'').

\bigskip

redpajama_set_name: RedPajamaArXiv


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redpajama_set_name: RedPajamaWikipedia


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Bumdiggibay
21 8 5 4 4 4 4 4 3 3 3 2 2 2 2 2 1 1 1 1 1 1 1 1 1 1 1 1 1 1 1 1 1 1 1 1 1 1


Backyard. Summer. A Child covered in bees.
Outside. Buzzing. Velcro shoes. Lurching. The crunch of grass.
Kitchen. Window. Mother. A glance.
Plates. Clatter. Feet. Scrambling. Screen door. Swinging.
Headspace. Memory. Intrusive. Mom as a girl. Florida. Home. A man. Inconsolable. His love. Swimming. Pulled under. A gator they said.
Whiskey. Guns. Man. Friends. A truck.
Horizon. An orange line. Dawn. Squealing brakes. Yelling. A crowd. Mother as child. Weaving. Men. Sweat. Flatbed. Full. Jagged shapes. Shovels. Wedging. Flatbed. Open. Dust. Wafting. The butcher's block sound of meat.
A pile. Alligators. Dead. The man. A knife. Tears. Ribbed bellies. A cut.
Her son. Collapsed. Face down. Blades of grass. Bees thinning. Skin. Pink. His head twice its size.
Fingers. Fumbling. Phone. 911. Operator. Please. My son.
A child. A baby. Her arms. His body. Her lap. Convulsing. Tremors. Breath. Her eyes. The sky. Virgin blue. And the clouds. Grand. Muscular. The clouds. Dinosaurs in the sky. The horizon. The trees. The wilderness. Beyond the pines. An ocean of lapse.


Well in a continuing series of unfortunate financial decisions I bought another Ascot today.
You may remember me from such Ascots as the one I already have with the Thumperstuff Header, Supertrapp exhaust, GSXR radial master cylinder and HEL braided lines.
Now I have this nightmare.
It's an 82. The ad didn't say it came with brake calipers and it didn't. Most of the wiring harness is missing. So are the side covers. The rear subframe is bent and the fork seals are blown out. So are the rear shocks. The handlebars are rusted through and I just spend the days staring at it pondering what brought me to this point in my life but I hope to make something out of it.
So if anyone has a decent condition wiring harness hit me up.
Kind of like rescuing a stray dog.
Good to see you back. Looking forward to seeing your progress.
Well, the van looks nice!
Good luck with the project. If it doen't work out, it's not as if you've ruined a reliable runner!


text:
La Norvège participe aux Jeux olympiques d'été de 1908 à Londres. 69 athlètes norvégiens ont participé aux compétitions dans aux sports. Ils y ont obtenu huit médailles : deux d'or, trois d'argent et trois de bronze.

Médailles

Voir aussi

Articles connexes

 Jeux olympiques d'été de 1908
 Norvège aux Jeux olympiques

Liens externes
  Norvège aux Jeux olympiques d'été de 1908 sur www.sports-reference.com
  Norvège sur le site du Comité international olympique
  Site officiel de la Fédération des sports de Norvège

Norvège
1908
1908 en Norvège


The double Dip Gate just barely fits into our "small gate" category. It is 1″ thick like all of our small gates and was one of our first attempts at using PVC for gates! It has been hanging since March of 2012 and looks as good today as when we first installed it, with no maintenance whatsoever!
Our PVC gates will withstand the weather requiring very little maintenance and last for years. Our gates are designed to be painted, or left as ordered. For PVC painting instructions, please click here.
Our small PVC gates are 1″ thick, and we provide information on what gate hardware to use. ( Allow for 1/4″ gap on either side of the gate. For $100 we will build a gate to fit your opening, as long as it is smaller than the gate described. Need a double gate? No problem – order 2!
The double Dip Gate just barely fits into our "small gate" category. It is 1″ thick like all of our small gates and was one of our first PVC gates! It has been hanging since March of 2012 and looks as good today as when we first installed it, with no maintenance whatsoever!


First day of Fall! . . First day of Fall!
My favorite time of the year is here & I couldn't be happier. The weather is still a little warm here but you can tell Fall weather is coming!
I told you on Tuesday that life has been SO busy ... & as if it weren't busy enough ... I may or may not have started yet another project in our home. Operation :: living room/foyer makeover ;). I mean, my hubby just loves me! HA! But after it's finished our entire downstairs will be all done! Yessssss!!
Besides painting, painting & a little more painting here is a look at what we've been up to . . .
Last week Millie Jo had her very first dentist appointment and rocked it just like I knew she would!
When did my girl get so big though?!?
Goodness gracious I love her!
You know your mama is a blogger when . . .
And please notice her tiny little toe trying to come out of her sandal :).
All the big, red, puffy heart emojis!
My little man had his second golf lesson on Monday afternoon & as I was watching him practice I was just amazed at how well he plays. He has been swinging a club since he was 3 years old & I pray everyday that God would use his talent if that's what Coop wants to do one day!
When his coach told the parents [there's only 5 in his class] to grab a golf cart, you can only imagine how excited these two were. They laughed the entire time riding on that thing!
And shout out to my hubby for taking Coop with him every time he goes & plays golf because he knew where to put his clubs & how to strap them on the back of the cart without me even having to help him!
This girl spent the hour of golf lessons turning flips.
When your daddy comes home from lunch & shares his peas with you.
Millie Jo is finally getting over her sinus infection & we are so happy about that. I have been enjoying all the extra snuggles!
On Tuesday morning, while Coop was at school, Dan took me & Millie Jo on a breakfast date. He let her pick where we went [as if he didn't already know where she wanted to go] & yep, you guessed it . . . Chickfila. The girl knows the way to my heart!
After breakfast we went to my second home lately Home Depot to get paint for my new said project.
Can't wait to share it with y'all soon plus my fall décor!
That's a little bit of this & that for you.
Before I go though, I want to ask y'all to say a special prayer for all police officers & their families. When I watch the news & see what's going on in Charlotte, NC it just breaks my heart. This world has become so heartbreaking & it's so scary to think what kind of world our children are growing up in.
This morning when I sat down to do my quiet time, I turned my devotional calendar to today & this is what it said . . .
For His anger is but for a moment, His favor for life; Weeping may endure for a night, but joy comes in the morning.
You just can't go wrong with Chick-fil-a! :) And, I felt the same way watching the news last night. Heartbreaking.


Arturia's MIDI controller line-up has grown considerably in recent years, from the affordable Keylab Essential 49 and 61 to the compact MiniLab MkIIs. The company's flagship KeyLab controllers, launched way back in 2013, were perhaps due for an update then, but the MkII models recently announced by Arturia are more than just a cosmetic update. Available in 49‑ and 61‑key formats, the Keylab MkII controllers feature a host of upgrades, including multi-coloured backlit pads, five expression control inputs and four CV outputs.
While the Keylab MkII's complement of controls is as generous as ever — with nine faders, nine rotary controllers and 16 performance pads, which can also trigger pre-programmed chords — Arturia are keen to stress that they haven't forgotten about the keyboard element of this controller keyboard. The MkII models come equipped with the same keybed as the exalted MatrixBrute synth, offering velocity and aftertouch and what Arturia describe as a luxurious playing feel.
In addition to the new CV outputs (pitch, gate and two modulation controllers) and expression control inputs (sustain, expression and three configurable aux inputs), Arturia have expanded the DAW control section, with 10 buttons that access common global and track-specific functions and a full set of transport controls. Arturia say that magnetic overlays will be included, allowing users to customise these controls for 10 of the most popular DAWs.
The Keylab MkIIs feature an all-aluminium chassis, with the same aluminium pitch bend and mod wheels seen on the MiniBrute 2 and real wood side panels. As we've come to expect, the new keyboards come bundled with some of Arturia's own virtual instruments, with both Piano V2 and Analog Lab 3 included. Due out in August, the Keylab MkII 49 will cost £399 and the Keylab MkII 61 will cost £439.


The innermost approached Tommy Yue to create a brand borchure that was different from other brands they saw in the product design. STEVE JONES wanted its brand to incorporate a more lifestyle element rather than just focusing on making money.
We were asked to do the brochure for innermost right after the shop launch. Their brochure is for product promotion. We have used artistic photo which is their brand images for the main visual.


A financial giant's recent foray into digital coin could mean increased cryptocurrency use — and its accompanying risks — in commercial banking.
Some 10 years ago Bitcoin became the world's first cryptocurrency, but mass adoption of it and other digital currencies has been hampered by price volatility and a general reluctance by investors, financial institutions, and regulators to get behind the technology. Barriers include lack of understanding about how the cryptocurrency works, as well as a trading process that can be opaque and subject to abuse — namely through hacking, market manipulation, and potential fraud.
That may be changing, however. In February JPMorgan Chase launched "JPM Coin," the first cryptocurrency created by a major U.S. bank. It will be used to settle payments between clients, and the lender will then work to transfer cross-border payments or corporate debt issuance services to the blockchain. The technology will facilitate near-instantaneous settlement of these money transfers and will, according to the bank, mitigate counterparty risk.
The move represents a dramatic change of attitude: Just a few years ago JPMorgan CEO Jamie Dimon called bitcoin a "fraud" and even threatened to fire employees who traded in it. Other banks, including HSBC, State Street, Credit Suisse, and Barclays, have either used blockchain and cryptocurrencies (albeit tentatively) or are planning to do so.
The committee said that crypto-assets "do not reliably provide the standard functions of money and are unsafe to rely on as a medium of exchange or store of value," adding that crypto-assets are not legal tender and are not backed by any government or public authority. Furthermore, the Basel Committee cited crypto-assets' history of volatility and lack of standardization and pointed to numerous risks it presents to banks, including liquidity risk, credit risk, market risk, operational risk, money laundering and terrorist financing risk, and legal and reputation risks.
Nonetheless, the committee accepts that banks may still want to participate in the crypto-market. As such, if a bank decides to acquire crypto-asset exposures or provide related services, it should adopt certain measures as a minimum — and internal auditors may want to take note.
Second, a bank's risk management framework for crypto-assets should be fully integrated into the overall risk management processes, including those related to anti-money laundering, combating the financing of terrorism and the evasion of sanctions, and heightened fraud monitoring. Furthermore, boards and senior management should be provided with timely and relevant information related to the bank's crypto-asset risk profile.
Third, a bank should publicly disclose any material crypto-asset exposures or related services as part of its regular financial disclosures. It should also specify the accounting treatment for such exposures, consistent with domestic laws and regulations.
Finally, the bank should inform its supervisory authority of actual and planned crypto-asset exposure or activity in a timely manner. Moreover, it should provide assurance that it has fully assessed the permissibility of the activity and the risks associated with the intended exposures and services, and explain how it has mitigated these risks.
In February QuadrigaCX gained worldwide media attention due to the unique circumstances surrounding its failure. After the death of its CEO Gerald Cotton, the collapsed exchange no longer had access to his laptop, which contained the keys for over US$100 million worth of customers' funds. And while the company's external auditor has since cracked the code, it found the funds had been transferred out of customers' crypto wallets in April 2018. The company's directors are still in the process of trying to pay off creditors, and many have accused QuadrigaCX of suspicious activity or at least extreme negligence. "It is safer to separate the assets across several private keys so that if a hack does occur or if a laptop goes missing, not all of the cryptocurrencies will be stolen or lost," says Wolfe.
Wolfe also warns that internal auditors should pay close attention to how crypto-assets are handled on the balance sheet. He points to the lack of standardization on cryptocurrency profit and loss treatment as a potential area of concern when reporting organizational value for tax purposes, particularly in light of current volatility.