He has been a wonderful actor and at a very early age he has been able to leave a mark. He is none other than the very talented Billy Unger. He was born in the year 1995 on 15th of October and this makes his age 19 at this time. At this age he has already faced paparazzi several times and his talent will guide him to the greatest heights soon. He was born in a place called Palm Beach County, which lies in Florida of United States of America. He belongs to the ethnicity white and nationality American. He is a tall man as he has a good height of 1.73 meters. The names of his parents are Karley Unger and William Unger and they must be very proud of what he has achieved in his career so far and they also know that he will grow even bigger in the industry. He has two siblings and their names are Eric Unger and Erin Unger.
As he has been so popular and so successful, information on him and his amazing biography can be grabbed from popular wiki sites such as Wikipedia and IMDb. He has a very impressive net worth of $400 thousand dollars and this proves how successful he has been in his career. He is also active in popular social networking sites such as Twitter and Instagram. He has a jaw dropping 230 thousand followers in Twitter and this proves how famous he has been in the site. He has already tweeted in the site more than 7 thousand times and this proves how involved he has been too. His Twitter account is verified as well. He has a very impressive 357 thousand followers in Instagram and he addresses them by uploading his hot pictures. He is a hunk and there is no doubt he looks red-hot when he goes shirtless. He has uploaded some of his shirtless pictures in Instagram as well.
He is not married right now and he does not have a wife. According to some sources he has been dating his girlfriend Angela Moreno from the year 2014 and their intimate affair has become one of the hottest topics of the town. If the couple goes strong, they might get engaged too. As he is dating a woman, he cannot be gay at all. Facts and relationships news related to him gets a lot of buzz. In the past he has already dated women like Raini Rodriguez, Allisun Ashley Arm and Teala Dunn.
He played the role of Frankie in a movie called Seven's Eleven: Sweet Toys in the year 2007 and this role of his is his movie debut. He also played the role of Charles Gates in a movie called National Treasure: Book of Secrets the same year. Other movies and TV shows to his credits up to now are Rock Slyde, Cop Dog, Tumbling, Sammy 2, The Love Forever, The Lost Medallion: The Adventures of Billy Stone, Desperate Housewives, Medium, Family Guy, Terminator: The Sarah Connor Chronicles and Mental.


Kiyonza is situated in a rural part of Southern Rwanda near the Burundi border. The aim of the project was to increase awareness, confidence and general life skills so that students would be better equipped to play an active role in society, support themselves and their families and use their new skills to help improve the infrastructure and skills base available in the job market.
At the time of our intervention, teachers were not being paid and students could only learn if they provided their own materials. Make a Difference 4 Africa worked with the Workforce Development Authority and the local mayor to identify what was needed to successfully develop the centre, ensure that students would gain a recognised certificate at the end of their studies and teacher salaries would be funded through local or national budgets.
Our first step was to renovate the existing buildings to make them fit for purpose and to provide tools, equipment, furniture and a small budget for the short-term running costs. We went on to provide better water facilities (there were no mains water facilities) and additional toilets. An income generation project and workers' cooperatives were then added to the mix and finally two new classrooms and a kitchen were built.
We successfully increased the number of places available to young people and turned a failing centre into one which the community and Make a Difference 4 Africa are justly proud.


text:
Tag "Impressions"
Battlefield V Open Beta impressions: What's all the fuss about?
The Battlefield V Open Beta just ended a few days ago. There is another article about it too, but I wanted to contribute to the conversation. There have been plenty
Battlefield 1 multiplayer hands-on preview
Shooter fans lately had been clamoring for a return to the World War II genre, and then DICE came out and said "We'll give you what you want… kind of."
Dishonored 2 hands-on impressions – Navigating a (literally) shifty mansion
Dishonored 2, Arkane Studios' sequel to its unique stealth-action game, is aiming to take the ideas presented from the first title and amplify them by 10. The night before I got a
Hands-on impressions of online shooter, LawBreakers
Thanks to Overwatch, my interest in online shooters has piqued, so it's no surprise that I jumped at the chance to play LawBreakers, the upcoming game from Gears of War creator Cliff Bleszinski's studio Boss Key
Theatrhythm Final Fantasy Impressions
I'm a sucker for music games. Anything having to do with tapping strings of notes in sync with the music often gives me a warm fuzzy feeling of knowing a

redpajama_set_name: RedPajamaCommonCrawl


text:
Q: Box positioning - cross-browser compatibility issue I have a problem with a page layout on the website I am working on.
Here's a link
The blue box on the right hand side is looking good in IE and Firefox, but it's too short (the text is too close to the bottom of the box) in Chrome, Safari and Opera.
Here's the code for the box:
#testimon {
   background: url("../img/ttm_bg.png") repeat-x scroll 0 0 transparent;
   border-radius: 15px 15px 15px 15px;
   border-top: 4px groove #00D1FA;
   box-shadow: 0 1px 4px 1px #555555;
   font-size: 14px;
   height: 788px;
   margin-top: 26px;
   padding: 3px;
   text-align: center;
   width: 262px;
 }
#testimon h4 {
   color: rgba(255, 255, 255, 0.92);
   font-size: 19px;
   margin: 8px 0 17px 0;
   text-shadow: 1px 2px 2px #1A1A1A;
 }
#testimon p {
   font-family:Georgia, "Times New Roman", Times, serif;
   color: rgba(0, 0, 0, 0.88);
   line-height:25px;
   font-size: 14px;
   font-style: oblique;
   font-weight: bold;
   text-shadow: 0 1px 1px #CCCCCC;
 }
#testimon .quote {
   font-size:25px;
   padding:4px;
 }
#testimon .signature {
   color: #e6e6e6;
   font-style: normal;
   margin-bottom: 15px;
   text-shadow: none;
 }
#testimon .spacer2 {
   background: url("../img/stars.png") no-repeat scroll 98px 0 transparent;
   height: 13px;
   margin: 31px 0 15px 0;
   width: 262px;
 }

Thanks for any help!

A: The problem is less a cross-browser issue and more a styling issue - you've got a fixed height on that testimonials div, so what if someone has different fonts than you specify, or increases the font size on their browser, the text will spill over (as it did when I upped the font using Firebug).
The solution is to remove the height from the #testimon element, and ensure that the background repeats vertically (which it currently does not).

A: This is probably a font rendering related issue.  The sizes are slightly different in each browser so the end overall height is different.  I would remove the height value from #testimon.

A: I look at the site with Crome, Opera, Maxathon, Firefox, Safari, and I.E., all browsers are current version of the browser. The images and the text look good. The only issue I could see were in some of the browsers you had to click on the image two or maybe three times to make the image to zoom in.
You might want to clear the cache of the browser and close and re-open the browser.

redpajama_set_name: RedPajamaStackExchange


text:
Frances Gertrude Claire D'Souza, Baroness D'Souza,  (née Russell; born 18 April 1944) is a British scientist and politician. She held the office of Lord Speaker from 1 September 2011 to 31 August 2016.

Early life, education and early career
Frances Gertrude Claire Russell, the daughter of Robert Anthony Gilbert and Pauline (née Parmet) Russell, was educated at St Mary's School, Princethorpe, and went to University College London to read anthropology, graduating BSc in 1970. She subsequently undertook further study at Lady Margaret Hall, Oxford, obtaining the degree of Doctor of Philosophy (D.Phil.) in 1976. She worked for the Nuffield Institute of Brain Chemistry and Human Nutrition from 1973 to 1977, Oxford Polytechnic (now Oxford Brookes University) from 1977 to 1980, and was an independent research consultant for the United Nations from 1985 to 1988. From 1989 to 2002, she was the director of the human rights organization Article 19. As its representative she supported the Musa Anter peace train to Diyarbakır, which aimed for peace in Kurdistan.

Personal life
In 1959, when she was 15, she married Dr Stanislaus Joseph D'Souza, with whom she had two children; they divorced in 1974. From 1985 to 1994 she was married to Martin John Griffiths. In 2003 she and D'Souza remarried. Their elder daughter is the journalist Christa D'Souza.

Honours
D'Souza was invested as a Companion of the Order of St Michael and St George in 1999.

House of Lords
D'Souza was created a Lord Temporal as Baroness D'Souza, of Wychwood in the County of Oxfordshire, on 1 July 2004. She sat as a crossbencher in the House of Lords, where she was the Convenor of the Crossbench Peers from 2007 to 2011 with attendance "well above average".

On 13 July 2011, D'Souza was elected Lord Speaker of the House of Lords and began her new role in September 2011.

In December 2015, the results of a Freedom of Information request revealed that D'Souza spent £230 to keep a chauffeured car waiting while she watched a performance of Benjamin Britten's Gloriana with the chairman of the Federation Council of Russia. The journey was just a mile from the Houses of Parliament. She spent £270 holding a car for four and a half hours while she had lunch with the Japanese ambassador in central London. It was also revealed that a 10-day official trip to Japan, Hong Kong and Taiwan in the autumn of last year cost nearly £26,000, and that she had spent £4,000 across a five-year period on fresh flowers for her office at the taxpayer's expense.

D'Souza's term as Lord Speaker ended on 31 August 2016. After returning to the crossbenches she called for urgent action to address the growing size of the House of Lords, including limits on the Prime Minister's patronage power.

References

External links

Baroness D'Souza on parliament.uk

1944 births
Living people
People educated at Princethorpe College
Alumni of University College London
Alumni of Lady Margaret Hall, Oxford
People from Sussex
People from Warwickshire
People from Oxfordshire
Academics of Oxford Brookes University
Companions of the Order of St Michael and St George
Crossbench life peers
Members of the Privy Council of the United Kingdom
People's peers
Lords Speaker
Life peeresses created by Elizabeth II

redpajama_set_name: RedPajamaWikipedia


text:
\section{Introduction}
The study of meson-baryon scattering is very important to understand
the properties of hadron resonances.
Because hadron resonances are short living and decay immediately by the strong interaction,
they appear only in the scattering processes and
one can deduce the properties of the hadron resonances only from the investigation of
the scattering process.
Description of scattering amplitude is one of the first steps to
investigate the hadronic resonances.
Once one obtains realistic scattering amplitudes reproducing the scattering cross sections
in terms of analytic functions, one can perform analytic continuation
to complex energy plane
and obtain properties of the resonances, such as
their masses, widths and coupling strengths.
For the purpose of description of the scattering amplitude in an analytic way,
one of the theoretical tools is the chiral effective theory in which
the low energy theorems by chiral symmetry constrain the hadronic interactions.
Chiral perturbation theory describes scattering amplitudes for the lowest channels, while
some unitarization procedure is necessary when one encounters resonances and open channels,
where hadronic dynamics plays an important role. For instance, chiral perturbation theory works
well for the $\pi N$ scattering at low energies, while, for the $\bar KN$ channel, since the
$\Lambda(1405)$ resonance is located in the $I=0$ channel below the threshold and the
$\pi\Sigma$ and $\pi\Lambda$ channels are open, one needs unitarization of the amplitude and
takes into account of coupled channels.

In this article, we reexamine the elastic scattering amplitude of $KN$ in low energies,
$p_{\rm lab}<800$ MeV/c, based on the chiral unitary approach
and study the possibility of an $S=+1$ exotic resonance in $I=0$ channel.
Baryons with strangeness $S=+1$ are so-called exotic hadrons, because
their quantum numbers cannot be described by three constituent quarks.
For the $S=+1$ baryon, one needs at least one anti-strange quark and more than three
quarks to compensate the negative baryon number of the anti-strange quark
to have baryon number $+1$ in total.
Thus, the minimal quark contents are $uudd\bar{s}$ for charge $Q=+1$.
Although there are no reasons to forbid the existence of such states
in quantum chromodynamics,
the experimental evidence for existence of the $S=+1$ baryons is not well confirmed.

The scattering amplitudes of the $K^{+}N$ scattering in low energies have been studied for a long time.
A comprehensive review can be found in Ref. \cite{dover1982}.
There are three $K^{+}N$ amplitudes, $K^{+}p \to K^{+}p$, $K^{+}n \to K^{+}n$ and $K^{+}n \to K^{0}p$
and isospin symmetry reduces two independent amplitudes for $I=0$ and $I=1$.
The $K^{+}p$ amplitude can be observed directly from the $K^{+}p \to K^{+}p$ scattering experiment
and provides the $I=1$ amplitude,
while for the $K^{+}n$ amplitudes one needs nuclear targets, such as deuterium,
and obtains the $I=0$ amplitude using the $I=1$ amplitude.
It is known that
the $K^{+}N$ scatterings are almost elastic for $p_{\rm lab} < 800$ MeV/c and inelastic contributions
are not significant~\cite{Bland:1969cb}.  For low energies, the $K^{+}p$ scattering is described
by $S$-wave~\cite{Goldhaber:1962zz}. In addition, the differential cross section of the $K^{+}p$ scattering
in low energies shows constructive interference between the Coulomb and strong interactions
at very forward angles. This implies that the low energy $K^{+}p$ scattering is to be repulsive~\cite{Goldhaber:1962zz,cameron1974}.
In contrast, the $I=0$ amplitude is more ambiguous.
In Refs.~\cite{Slater:1961zz,PhysRev.134.B1111},
it was shown that the scattering amplitude for $I=0$ has $P$-wave contribution
to reproduce the $K^{+}d$ scattering up to $p_{\rm lab} < 500$ MeV/c.
The phase shift analysis up to $1.5$ GeV/c by Ref.~\cite{Giacomelli:1974az} found several solutions,
in which one solution implies that the low energy scattering is described dominantly by $S$-wave,
while another solution reproduces the amplitude mainly by $P$-wave.
The phase shift analyses with new data performed by Refs.~\cite{Sakitt:1975hu,Sakitt:1976ny,Glasser:1977xs}
supported the latter $P$-wave solution.
The analysis carried out by Ref.~\cite{martin1975} treated
both $I=0$ and $I=1$ amplitudes at the same time,
and found that the $P$-wave contribution was significant for the low energy $I=0$ amplitude.

The search for $S=+1$ resonance has been carried out in the past.
In the earlier studies,
a possible $S=+1$ broad resonance $Z^{\ast}$ in the $KN$ scattering with $I=0$
were discussed~\cite{Cool:1966zz,Tyson:1967zz,bugg1968,abrams1969,Giacomelli:1972uj,wilson1972,Giacomelli:1973ed,carroll1973,Giacomelli:1974az}.
In Ref.~\cite{abrams1969}, it was pointed out that there the $K^{+}N$ total cross
sections \cite{Cool:1966zz} and $K^{-}$ photoproduction \cite{Tyson:1967zz} showed
two bump structures which would have risen possible $KN$ resonances with $I=0$.
Although the phase shift analysis by Martin~\cite{martin1975} found that there were
no significant resonances in the partial wave amplitude, the Argand diagram suggested
that there could be some broad resonances appearing in $P_{01}$ and $D_{03}$ \cite{Lea:1968,Watts:1980qs,Robertson:1980ma}.
These resonances were reported as broad resonances above
the energies where the inelastic contributions start to be significant.
The studies of the bump structure in cross sections and the behavior of the Argand diagrams
are not sufficient to fix the existence of the resonance states. One of the promising ways
is to analyze the scattering amplitude as a analytic function and to carry out analytic continuation
of the amplitude into the complex energy plane. Resonance states are expressed as poles of the
scattering amplitude.
Another kind of the resonance with $S=+1$ was suggested by LEPS collaboration
in photoproduction experiments~\cite{nakano}. They claimed a narrow resonance, $\Theta^{+}$,
with $S=+1$ and 1.5 GeV/${\rm c}^{2}$ mass~\cite{nakano,Nakano:2008ee}.
This experiment was motivated by a theoretical work \cite{diakonov}
predicting a resonance with $S=+1$ around the mass 1540 MeV/${\rm c}^{2}$ and narrow width $\Gamma < 15$ MeV.
Further studies in the chiral soliton model were performed in Refs. \cite{jaffe, weigel}.
The $\Theta^{+}$ resonance is obviously different from the previous $Z^{\ast}$ resonance.
Here we revisit the possibility of the existence of a $Z^{*}$-type
broad resonance with $S=+1$ and $I=0$
at lower energies than where the inelastic contributions start to be significant.

As mentioned in the above, it is important to understand the resonance properties by
studying the scattering amplitude, especially in terms of an analytic function.
There are several approaches to describe baryon resonance.
We use chiral unitary model, in which scattering problem is solved in a simplified manner
by considering elastic unitarity of the two-body scattering and the elementary interaction
is given based on chiral perturbation theory, firstly suggested in Ref. \cite{kaiser1995} and
developed in \cite{oset1998}, for the $S=-1$ channel,
and we can find recent progress in a review article~\cite{hyodo2012}.
Chiral unitary model impose unitary condition by infinite summation of the specific diagram
and describes the scattering amplitude as an analytic function.
Thus, it is easy to perform analytic continuation of the scattering amplitude
and to pin down the position of the resonance state in the complex energy plane.
One of the most successful examples of this approach is the finding of the
double pole structure of the $\Lambda(1405)$ and investigation of
its physical significance~\cite{Oller:2000fj,Jido:2003cb}.
It was reported in Refs.~\cite{Hyodo:2006yk,Hyodo:2006kg} that the Tomozawa-Weinberg interactions
for the exotic channels do not provide enough attraction to make two-body bound states
for a Nambu-Goldstone boson and a hadron. Actually the Tomozawa-Weinberg term vanishes
for $I=0$ and $S=+1$. Here the next-to-leading contributions are responsible for the attraction
to provide a broad resonance.

This paper is organized as follows.
In Sec. \ref{sec:sec2}, we construct $KN$ scattering amplitude using chiral perturbation theory
and chiral unitary model.
In Sec. \ref{sec:sec3}, we determine the parameters which reproduce $KN$ scattering data.
The total cross section and differential cross section data are compared with our results.
Using the constructed amplitude, we discuss the possibility of resonance with large width.
In Sec. \ref{sec:sec4}, we summarize the results of this paper.

\section{Formulation}
\label{sec:sec2}
For our theoretical investigation, we would like to represent the $KN$ scattering amplitude
in an analytic function of the center of mass energy $W$. Once we parametrize
the scattering amplitude in an analytic function,  analytic continuation allows us
to extend the amplitude to the complex energy plane, where resonances
are represented as poles, and extract the properties of resonances,
such as mass, decay width and coupling strength.
For this purpose, we describe the $KN$ elastic scattering amplitude based on the chiral unitary approach by solving
Lippmann-Schwinger equation
\begin{equation}
    T = V + VGT
\end{equation}
in a simplified way. In the chiral unitary approach,
the interaction kernel $V$ is given by chiral perturbation theory and
we restrict the intermediate state to the elastic channel.
The model parameters are determined so as to reproduce the observed $KN$ cross section.

\subsection{Scattering amplitude}
\label{sec:amp}

Let us call the momenta of the kaon and nucleon in the initial (final) state
by $p_{1}$ and $p_{2}$ ($p_{3}$ and $p_{4}$), respectively. According to Lorentz invariance,
the $T$-matrix of the $KN$ scattering can be written in terms of two Lorentz invariant functions,
$A(s,t)$ and $B(s,t)$, in general, as
\begin{equation}
  T(s,t) = \bar u (\vec p_{4},s_{4}) \left[A(s,t) + \frac12(p \hspace{-5pt}/ _{1}+p \hspace{-5pt}/ _{3}) B(s,t) \right] u(\vec p_{2},s_{2})
\end{equation}
with the Mandelstam variables $s=(p_{1}+p_{2})^{2}$ and $t=(p_{1}-p_{3})^{2}$ and
the on-shell Dirac spinor $u(\vec p, s)$ for nucleon with momentum $p$ and spin $s$. The Dirac spinor $u(\vec p, s)$ is normalized by $\bar u(\vec p,s) u(\vec p,s^{\prime}) = 2M_{N} \delta_{ss^{\prime}}$ with the nucleon mass $M_{N}$.
For partial wave decomposition, we write the $T$-matrix in the center of mass system
with two functions $f$ and $g$ in terms of the spin-nonflip and spin-flip parts as
\begin{equation}
  T(s,t)
   = \chi^{\dagger}(\lambda_{4})\left[ f(W,\theta) - i (\vec \sigma \cdot \hat n) g(W,\theta)\right]
   \chi(\lambda_{2})
\end{equation}
where $W$ and $\theta$ are the total energy and scattering angle (angle between $\vec p_{1}$ and $\vec p_{3}$)
in the center of mass system, respectively, $\hat n$ is the normal vector of the scattering plane
defined by $\hat n = (\vec p_{3} \times \vec p_{1})/ | \vec p_{3} \times \vec p_{1}|$, and
$\chi(\lambda)$ is Pauli spinor of nucleon with helicity $\lambda$.
The relation between $A, B$ and $f, g$ in the $KN$ elastic scattering is given by
\begin{eqnarray}
   f(W,\theta) &=&  (E_{N}+M_{N}) (A + \omega B )
   + k^{2} B
   +  \frac{(E_{N}+M_{N}+\omega)B-A}{E_{N}+M_{N}} k^{2} \cos\theta, \\
   g(W, \theta) &=& \frac{A- (E_{N} + M_{N} + \omega)B}{(E_{N}+M_{N})} k^{2} \sin\theta
\end{eqnarray}
with the kaon energy $\omega$, the 3-momentum in the center of mass system $k$ and
the nucleon energy $E_{N}$.

The amplitudes $f(W,\theta)$ and $g(W,\theta)$ can be decomposed into partial waves with
Legendre polynomials $P_{\ell}(x)$ as
\begin{eqnarray}
   f(W,\theta) &=& \sum_{\ell=0}^{\infty} f_{\ell}(W) P_{\ell}(\cos\theta) ,\\
   g(W,\theta) &=& \sum_{\ell=1}^{\infty} g_{\ell}(W) \sin\theta \frac{dP_{\ell}(\cos\theta)}{d\cos\theta}.
\end{eqnarray}
It is convenient to introduce the amplitude $T_{\ell \pm}$ having definite total angular momentum
$j=\ell \pm \frac12$ by
\begin{eqnarray}
   f_{\ell}(W) &=& (\ell+1) T_{\ell+}(W) + \ell T_{\ell-}(W), \\
   g_{\ell}(W) &=& T_{\ell+} (W) - T_{\ell-}(W),
\end{eqnarray}
or equivalently
\begin{eqnarray}
    T_{\ell+}(W) &=&  \frac{1}{2\ell+1} (f_{\ell} (W) + \ell g_{\ell}(W)), \\
    T_{\ell-}(W) &=& \frac{1}{2\ell +1} (f_{\ell}(W) - (\ell+1) g_{\ell}(W)).
\end{eqnarray}
We also introduce the partial-wave decomposed interaction kernels $V_{\ell+}(W)$ and $V_{\ell-}(W)$
in the same way.

Here we show the $KN$ scattering amplitudes in the isospin channels, $T^{I=0}$ and $T^{I=1}$.
The amplitudes in the particle basis can be obtained as
\begin{eqnarray}
    T_{K^{+}p \to K^{+}p} &=& T^{I=1}, \\
    T_{K^{+}n \to K^{+}n} &=& \frac{1}{2} (T^{I=1} + T^{I=0}), \label{eq:Kn} \\
    T_{K^{+}n \to K^{0}p} &=& \frac{1}{2} (T^{I=1} - T^{I=0}). \label{eq:CE}
\end{eqnarray}

Taking spin average in the initial state and spin summation in the final state
for nucleon,
we calculate the differential cross section in the center of mass frame as
\begin{equation}
   \frac{d \sigma}{d \Omega} = \frac{1}{64 \pi^{2} s} \left( |f(W,\theta)|^{2} + |g(W,\theta)|^{2} \right)
\end{equation}
and the total cross section by integrating the differential cross section in terms of the scattering angle as
\begin{equation}
  \sigma = \frac{1}{32 \pi s} \int_{-1}^{1} d\cos\theta \left( |f(W,\theta)|^{2} + |g(W,\theta)|^{2} \right).
\end{equation}

\subsection{Chiral Lagrangian}

The leading order chiral Lagrangian for the baryon field $B$ reads
\begin{eqnarray}
{\cal L}_{MB}^{(1)}=
{\rm Tr} \left[\bar{B}(i D \hspace{-7pt} / \, - M_{0}) B\right]
- \frac{D}{2} {\rm Tr} \left(\bar{B} \gamma_{\mu} \gamma_{5} \{u^{\mu},B\} \right)
-\frac{F}{2} {\rm Tr} \left (\bar{B} \gamma_{\mu} \gamma_{5} [u^{\mu},B] \right)
\label{eq:MB_1},
\end{eqnarray}
where $M_{0}$ is the baryon mass at the chiral limit,
the baryon and meson fields, $B$ and $\Phi$, are written in the SU(3) matrix form
\begin{eqnarray}
B&=&\left(
\begin{array}{ccc}
\frac{\Sigma^{0}}{\sqrt{2}}+\frac{\Lambda}{\sqrt{6}} &\Sigma^{+}& p \\
\Sigma^{-} & -\frac{\Sigma^{0}}{\sqrt{2}}+\frac{\Lambda}{\sqrt{6}} & n \\
\Xi^{-}& \Xi^{0} &  -\frac{2\Lambda}{\sqrt{6}}
\end{array}
\right), \\
\Phi&=&\left(
\begin{array}{ccc}
\frac{\pi^{0}}{\sqrt{2}}+\frac{\eta}{\sqrt{6}} & \pi^{+} &K^{+} \\
\pi^{-} & -\frac{\pi^{0}}{\sqrt{2}}+\frac{\eta}{\sqrt{6}} & K^{0} \\
K^{-}& \bar{K}^{0} &  -\frac{2\eta}{\sqrt{6}}
\end{array}
\right).
\end{eqnarray}
We parametrize the chiral field $U$ in the CCWZ form as
\begin{equation}
   U = \xi^{2} = \exp \left( i \frac{\sqrt 2}{f} \Phi\right)
\end{equation}
with a scale parameter $f$, which is turned to be identified as the meson decay constant in the leading order
calculation of chiral perturbation theory,
the covariant derivative for the baryon field is introduced as
\begin{equation}
   D_{\mu} B= \partial_{\mu} B + [ \Gamma_{\mu}, B ],
\end{equation}
with the mesonic vector current
\begin{equation}
   \Gamma_{\mu} = \frac{1}{2} ( \xi^{\dagger} \partial_{\mu} \xi + \xi \partial_{\mu} \xi^{\dagger} ),
\end{equation}
and the meson-baryon coupling is given through the mesonic axial vector current
\begin{equation}
   u_{\mu} = i \left(\xi^{\dagger} \partial_{\mu} \xi - \xi \partial_{\mu} \xi^{\dagger} \right)
\end{equation}
with low energy constants $D$ and $F$. The parameters $D$ and $F$ are to be determined
by the axial couplings of the baryons at tree level.

The next-leading order of the chiral Lagrangian
is composed of several terms
\begin{align}
{\cal L}_{MB}^{(2)}
=&b_{D} {\rm Tr} \left(\bar{B} \{ \chi_{+}, B \} \right)
+b_{F} {\rm Tr} \left(\bar{B} [\chi_{+}, B] \right)
+b_{0} {\rm Tr} (\bar{B}B) {\rm Tr} (\chi_{+})
+d_{1} {\rm Tr} \left(\bar{B} \{ u_{\mu}, [u^{\mu}, B] \} \right)
\nonumber \\ &
+d_{2} {\rm Tr} \left(\bar{B} [u_{\mu}, [u^{\mu}, B]] \right)
+d_{3} {\rm Tr} \left(\bar{B} u_{\mu} ) {\rm Tr} (u^{\mu} B \right)
+d_{4} {\rm Tr} \left(\bar{B} B) {\rm Tr} (u^{\mu} u_{\mu} \right)
\nonumber \\
&-\frac{g_{1}}{8M_{N}^{2}} {\rm Tr}  \left( \bar B \{ u_{\mu}, [ u_{\nu}, \{D^{\mu},D^{\nu}\}B] \} \right)
-\frac{g_{2}}{8M_{N}^{2}} {\rm Tr}  \left( \bar B [ u_{\mu}, [ u_{\nu}, \{D^{\mu},D^{\nu}\}B] ] \right)
\nonumber \\
&-\frac{g_{3}}{8M_{N}^{2}} {\rm Tr}  (\bar B  u_{\mu} ) {\rm Tr}  ( u_{\nu}, \{D^{\mu},D^{\nu}\}B)
-\frac{g_{4}}{8M_{N}^{2}} {\rm Tr}  (\bar B\{D^{\mu},D^{\nu}\}B) {\rm Tr} (u_{\mu} u_{\nu})
\nonumber \\
&-\frac{h_{1}}{4} {\rm Tr}  \left( \bar B [\gamma^{\mu},\gamma^{\nu}] B u_{\mu} u_{\nu} \right)
-\frac{h_{2}}{4} {\rm Tr}  \left( \bar B [\gamma^{\mu},\gamma^{\nu}] u_{\mu} [u_{\nu}, B] \right)
\nonumber \\
&-\frac{h_{3}}{4} {\rm Tr}  \left(\bar B [\gamma^{\mu},\gamma^{\nu}] u_{\mu} \{u_{\nu}, B\} \right)
-\frac{h_{4}}{4} {\rm Tr}  (\bar B [\gamma^{\mu},\gamma^{\nu}] u_{\mu}) {\rm Tr} (u_{\nu} B) + {\rm h.c.}
\label{eq:MB_2}
\end{align}
where $b_{i}$, $d_{i}$, $g_{i}$ and $h_{i}$ are low energy constants.
The terms with $b_{i}$ and $d_{i}$ appear in the typical SU(3) chiral Lagrangians,
while the terms with $g_{i}$ and $h_{i}$ are introduced as an extension of the SU(2) chiral Lagrangian \cite{Bernard:1995dp,Fettes:2000gb}. (See also Ref.~\cite{Lutz:2001yb}.)
The scalar field $\chi_{+}$ is given by
\begin{equation}
   \chi_{+} = 2 B_{0} \left (\xi {\cal M} \xi + \xi^{\dagger} {\cal M} \xi^{\dagger} \right),
\end{equation}
with the quark mass matrix
\begin{equation}
    {\cal M}={\rm diag} \left(\hat{m}, \hat{m}, m_{s} \right),
\end{equation}
where $\hat m$ stands for the mass of the $u$ and $d$ quarks by assuming isospin symmetry,
while $m_{s}$ means the strange quark mass.
Parameter $B_{0}$ is a positive constant related to the meson mass and always appears
together with the quark mass.
The parameter is fixed by $B_{0}=M_{K}^{2}/(\hat{m}+m_{s})$ where $M_{K}$ is the kaon mass.
The low energy constants some combinations of
$b_{i}$, $d_{i}$, $g_{i}$ and $h_{i}$ are to be fixed
by the $KN$ scattering cross sections.

\subsection{Interaction kernel}

The tree level amplitude of the $KN$ scattering up to the next-to-leading order
is composed by three parts, the leading order contact term, the hyperon crossed Born term,
and the next-to-leading contact term.
The leading order contact term is called Tomozawa-Weinberg term,
and is determined by the SU(3) group structure of hadrons
without the low energy constants. It is known to be absent for the $KN$ channel with $I=0$:
\begin{eqnarray}
   V^{I=0}_{\rm TW} = 0, \qquad
   V^{I=1}_{\rm TW} = \frac{1}{2f_{K}^{2}}
   \bar{u}(\vec{p}_4,s_4)(p \hspace{-5pt}/ _1+p \hspace{-5pt}/ _{3}) u(\vec{p}_2,s_2).
\end{eqnarray}
The corresponding invariant amplitudes read
\begin{eqnarray}
  A^{I=0}_{\rm TW} = B^{I=0}_{\rm TW} = A^{I=1}_{\rm TW} = 0, \qquad
  B^{I=1}_{\rm TW} = \frac{1}{f_{K}^{2}}.
\end{eqnarray}
For the Born term, we do not consider explicit baryonic states with strangeness $S=+1$.
The pentaquark $\Theta^{+}$ is a candidate for such a state, but it is known to have a
narrow width and a very weak coupling to $KN$. The hyperons with $S=-1$, $\Sigma$ and $\Lambda$,
contribute to the $KN$ amplitude as crossed Born terms.
With the chiral Lagrangian (\ref{eq:MB_1}), we obtain the crossed Born terms as
\begin{eqnarray}
V^{I=0}_{{\rm Born}}&=& -\frac{3}{4}\frac{(D-F)^{2}}{f^{2}_{K}}
\bar{u}(\vec{p}_4,s_4)p \hspace{-5pt}/ _1\gamma_5
\frac{M_{\Sigma} + (p \hspace{-5pt}/ _2 - p \hspace{-5pt}/ _3) }{M_{\Sigma}^{2} - (p_{2} - p_{3} )^{2} - i\epsilon}
p \hspace{-5pt}/ _3\gamma_5u(\vec{p}_2,s_2)
\nonumber\\
&&+\frac{1}{12} \frac{(3F+D)^{2}}{f^{2}_{K}}\bar{u}(\vec{p}_4 ,s_4)p \hspace{-5pt}/ _1\gamma_5
\frac{M_{\Lambda} + (p \hspace{-5pt}/ _2 - p \hspace{-5pt}/ _{3}) }{M_{\Lambda}^{2} - (p_{2} - p_{3} )^{2} - i\epsilon}
p \hspace{-5pt}/ _3\gamma_5u(\vec{p}_2,s_2), \label{eq:I02} \\
V^{I=1}_{\rm Born} &=&  -\frac{1}{4} \frac{(D-F)^{2}}{f^{2}_{K}}
\bar{u}(\vec{p}_4,s_4)p \hspace{-5pt}/ _1\gamma_5
\frac{M_{\Sigma} + (p \hspace{-5pt}/ _2 - p \hspace{-5pt}/ _{3}) }{M_{\Sigma}^{2} - (p_{2} - p_{3} )^{2} - i\epsilon}
p \hspace{-5pt}/ _3\gamma_5 u(\vec{p}_2,s_2)
\nonumber\\
&&-\frac{1}{12}\frac{(3F+D)^{2}}{f^{2}_{K}}\bar{u}(\vec{p}_4 ,s_4)p \hspace{-5pt}/ _1\gamma_5
\frac{M_{\Lambda} + (p \hspace{-5pt}/ _2 - p \hspace{-5pt}/ _{3} ) }{M_{\Lambda}^{2} - (p_{2} - p_{3} )^{2} - i\epsilon}
p \hspace{-5pt}/ _3\gamma_5u(\vec{p}_2,s_2) \label{eq:I12}
\end{eqnarray}
with the $\Sigma$ mass $M_{\Sigma}$ and $\Lambda$ mass $M_{\Lambda}$.
The invariant amplitudes are written as
\begin{eqnarray}
   A^{I=0}_{\rm Born} &=& \frac34 \frac{(D-F)^{2}}{f^{2}_{K}}
     \frac{(M_{N}+M_{\Sigma})(M_{N}^{2}-u)}{u - M_{\Sigma}^{2}}
    -\frac{1}{12} \frac{(3F+D)^{2}}{f^{2}_{K}}
    \frac{(M_{N}+M_{\Lambda})(M_{N}^{2} - u)}{u - M_{\Lambda}^{2}},
     \\
   B^{I=0}_{\rm Born} &=& -\frac34 \frac{(D-F)^{2}}{f^{2}_{K}}
    \frac{u+M_{N}^{2} + 2 M_{\Sigma} M_{N} }{u - M_{\Sigma}^{2}}
    +\frac{1}{12} \frac{(3F+D)^{2}}{f^{2}_{K}}
    \frac{u+M_{N}^{2} +2 M_{\Lambda} M_{N}}{u - M_{\Lambda}^{2}},\\
   A^{I=1}_{\rm Born} &=& \frac14 \frac{(D-F)^{2}}{f^{2}_{K}}
     \frac{(M_{N}+M_{\Sigma})(M_{N}^{2}-u)}{u - M_{\Sigma}^{2}}
    +\frac{1}{12} \frac{(3F+D)^{2}}{f^{2}_{K}}
    \frac{(M_{N}+M_{\Lambda})(M_{N}^{2} - u)}{u - M_{\Lambda}^{2}},
     \quad \\
   B^{I=1}_{\rm Born} &=& -\frac14 \frac{(D-F)^{2}}{f^{2}_{K}}
    \frac{u+M_{N}^{2} + 2 M_{\Sigma} M_{N} }{u - M_{\Sigma}^{2}}
    -\frac{1}{12} \frac{(3F+D)^{2}}{f^{2}_{K}}
    \frac{u+M_{N}^{2} +2 M_{\Lambda} M_{N}}{u - M_{\Lambda}^{2}}
\end{eqnarray}
with Mandelstam variable $u = (p_{1}-p_{4})^{2} = 2M_{N}^{2}+2M_{K}^{2} - s -t $,
the nucleon mass $M_{N}$ and the kaon mass $M_{K}$.
The $KN$ invariant amplitudes at the next-to-leading order chiral perturbation theory
are calculated for each isospin channel as
\begin{eqnarray}
V^{I}_{\rm NLO}&=&
\left[
\frac{4B_0}{f^{2}_{K}}(\hat{m}+m_s)b^{I}
+\frac{2}{f^{2}_{K}}  (p_1\cdot p_3) d^{I}
 \right .\nonumber \\ && \quad \left.
+\frac{(p_{2}\cdot p_{1})(p_{2}\cdot p_{3}) + (p_{4}\cdot p_{1})(p_{4}\cdot p_{3})}{2M_{N}^{2} f_{K}^{2}} g^{I}
\right]
\bar{u}(\vec{p}_4,s_4)u(\vec{p}_2, s_2)
\nonumber \\ &&
 - \frac{ h^{I}}{2f_{K}^{2}}  p_{1}^{\mu} p_{3}^{\nu}\,  \bar{u}(\vec{p}_4,s_4) [\gamma_{\mu}, \gamma_{\nu}]
u(\vec{p}_2, s_2),
 \label{eq:I03}
\end{eqnarray}
and the corresponding invariant amplitudes $A$ and $B$ read
\begin{eqnarray}
   A_{\rm NLO}^{I} &=& \frac{4B_0}{f^{2}_{K}}(\hat{m}+m_s)b^{I}
+\frac{2}{f^{2}_{K}}  (p_1\cdot p_3) d^{I}
  \nonumber \\ &&
+\frac{(p_{2}\cdot p_{1})(p_{2}\cdot p_{3}) + (p_{4}\cdot p_{1})(p_{4}\cdot p_{3})}{2M_{N}^{2} f_{K}^{2}} g^{I}
+ \frac{p_{1}\cdot(p_{2}+p_{4})}{f_{K}^{2}} h^{I}\\
   B_{\rm NLO}^{I} &=& -\frac{2 M_{N}}{f_{K}^{2}} h^{I}.
\end{eqnarray}
In these equations, the parameters $b^{I}$, $d^{I}$, $g^{I}$ and $h^{I}$ are defined by
\begin{align}
  b^{I=0} &= b_{0} - b_{F},                    & b^{I=1} &= b_{0} + b_{D}, \\
  d^{I=0} &= 2d_{1} + d_{3} - 2d_{4},    & d^{I=1} &= -2d_{2} - d_{3} - 2d_{4}, \\
  g^{I=0} &=  2g_{1} + g_{3} - 2 g_{4},   & g^{I=1} &=  -2g_{2} - g_{3} - 2 g_{4}, \\
  h^{I=0} &= h_{1}+h_{2}+h_{3}+h_{4},    & h^{I=1} &= h_{1}-h_{2}-h_{3}-h_{4},
\end{align}
in terms of the low energy constants appearing in Lagrangian (\ref{eq:MB_2}).
We treat these combinations of the low energy constants as free parameters
to be adjusted to reproduce observed $KN$ cross sections.

\subsection{Unitarization}

Unitarization is performed in each partial wave amplitude~\cite{Jido:2002zk}.
Because the total angular momentum is a good quantum number, Lippmann-Schwinger equation is also
decomposed into partial waves as
\begin{equation}
   T_{\ell \pm}^{I} = V_{\ell \pm}^{I} + V_{\ell \pm}^{I} G T_{\ell \pm}^{I}
\end{equation}
where we have assume that we use a non-relativistic Green's function and do not consider
so-called zig-zag diagrams which mix the large and small components of the Dirac spinor.
Supposing that we take only the on-shell contribution of the interaction kernel
in the loop integral, we can solve Lippmann-Schwinger equation algebraically
\begin{equation}
\label{eq:less_amp}
   T_{\ell \pm}^{I} = (1 - V_{\ell \pm}^{I}G)^{-1} V_{\ell \pm}^{I}
\end{equation}
where the loop contribution $G$ for the $KN$ channel is given
as a function of the center of mass energy, $W$, by
\begin{equation}
   G(W) = i\int \frac{d^{4} q}{(2\pi)^{4}} \frac{1}{(P-q)^{2} - M_{N}^{2} + i \epsilon}
   \frac{1}{q^{2} - M_{K}^{2} + i \epsilon} .
\end{equation}
This integral can be
performed by the dimensional regularization as
\begin{eqnarray}
G(W)&=&\frac{1}{(4 \pi )^{2}}
\biggl \{ a(\mu)
+\ln \frac{M_{N}^{2}}{\mu^{2}}
+\frac{M_{K}^{2}-M_{N}^{2} +s}{2 s} \ln \frac{M_{K}^{2}}{M_{N}^{2}}  \nonumber \\
&&+\frac{k}{\sqrt{s}} \Bigl [ \ln(s - (M_{N}^{2} - M_{K}^{2})
+ 2\sqrt{s} k) + \ln \left(s + \left(M_{N}^{2} - M_{K}^{2} \right) +2\sqrt{s} k \right) \nonumber \\
&&-\ln \left(-s + \left(M_{N}^{2} - M_{K}^{2} \right)
+2\sqrt{s} k \right)
-\ln\left(-s-\left(M_{N}^{2}-M_{K}^{2}\right)
+2\sqrt{s} k \right) \Bigl]  \biggl \},
\label{eq:loop}
\end{eqnarray}
where $\mu$ is the scale parameter of the dimensional regularization and
$a(\mu)$ is the subtraction constant depending on $\mu$.
We take away the infinite part as renormalization procedure, and
the subtraction constant is determined so as to reproduce experiments.
For the interaction kernel, here we take the chiral perturbation amplitudes
calculated in the previous section up to the next-to-leading order as
\begin{equation}
    V^{I} = V_{\rm WT}^{I} + V_{\rm Born}^{I} + V_{\rm NLO}^{I}
\end{equation}
and perform partial wave decomposition in the way explained in Sec.~\ref{sec:amp}.

\subsection{Coulomb correction}
For the $K^{+}p$ amplitude, we introduce the Coulomb correction
as done in Ref.~\cite{hashimoto}.
To the strong interaction part of the $K^{+}p$ scattering amplitude
calculated in the center of mass frame,
we add
the Coulomb amplitude
\begin{equation}
  f_{C} = -\frac{\alpha}{2 k v \sin^{2}(\theta/2)} \exp\left[ - i \frac{\alpha}{v}
  \ln \left(\sin^{2} \frac{\theta}{2} \right)\right]
\end{equation}
with the scattering angle $\theta$, the fine structure constant $\alpha$
and the $KN$ relative velocity $v$ defined by
\begin{equation}
  v = \frac{ k (E_{K} + E_{p})}{E_{K}E_{p}},
\end{equation}
and multiply the Coulomb phase shift factor $e^{2i \Phi_{\ell}}$
with
\begin{equation}
   \Phi_{\ell} = \sum_{n=1}^{\ell} \tan^{-1} \frac{\alpha}{n v}
\end{equation}
for $\ell >0$ ($\Phi_{0} = 0$) as
\begin{eqnarray}
   f^{K^{+}p} &=& \sum_{\ell=0}^{\infty} \left[ (\ell+1) T_{\ell+}^{I=1}
   + \ell T_{\ell-}^{I=1} \right] e^{2i\Phi_{\ell}} P_{\ell}(\cos\theta)
   - 8 \pi \sqrt s f_{C}, \\
   g^{K^{+}p} &=& \sum_{\ell=1}^{\infty}
   \left[T_{\ell+}^{I=1} - T_{\ell-}^{I=1}\right]    e^{2i\Phi_{\ell}}
   \sin\theta \frac{dP_{\ell}(\cos\theta)}{d\cos\theta} .
\end{eqnarray}

\section{Results}
\label{sec:sec3}

In the previous section, we have constructed the unitarized $KN$ amplitudes using the chiral unitary model.
In this section, we carry out the $\chi^{2}$ fitting of the unitarized amplitude to the experimental data
and determine the low-energy constants appearing in the next-to-leading order.
We assume to fix the subtraction constants for $I=0$ and $1$ at $a^{I=0,1} = -1.150$
with the regularization scale $\mu=1$ GeV
to suppress the number of the parameters in the situation that the experimental data have somewhat large error
and disagreement in different experiments.
Moderate change of the subtraction constants can be absorbed into the low-energy constants.
We assume isospin symmetry and use the isospin averaged masses for the hadrons.
We take the kaon decay constant as $f_{K} = (1.19 \pm 0.01)f_{\pi} = 110.0$ MeV where $f_{\pi}$ = 92.4 MeV.
The low-energy constants at the leading-order chiral Lagrangian $D$ and $F$
are already determined by the semileptonic hyperon beta decay reported in \cite{DandF} as
\begin{eqnarray}
D=0.80, \enspace F= 0.46.
\end{eqnarray}
The values of these parameters are summarized in Table~\ref{tab:masses}.

\begin{table}[t]
\begin{center}
\caption{The values of the fixed parameters. We take the isospin averaged masses. }
\label{tab:masses}
\begin{tabular}{ccccccc}
\hline
$M_{N}$ & $M_{K}$ & $M_{\Lambda}$ & $M_{\Sigma}$ & $f_{K}$ & $D$ & $F$ \\
\hline\hline
$938.9$ MeV & $495.6$ MeV & $1115.7$ MeV & $1193.2$ MeV & $110.0$ MeV & 0.80 & 0.46 \\
\hline
\end{tabular}
\end{center}
\end{table}

\subsection{Determining amplitude}
We determine the $KN$ amplitudes for $I=1$ and $I=0$
reproducing the experimental data using the $\chi^{2}$ fitting of the low-energy constants to minimize
the $\chi^{2}$ function
\begin{eqnarray}
\chi^{2} = \sum_{i}^{N} \left(\frac{y_{i} - f(x_{i})}{\sigma_{i}} \right)^{2},
\end{eqnarray}
where $y_{i}, f(x_{i}), \sigma_{i}$ and $N$ are the experimental data,
the theoretical calculations with the parameters, the errors of the data and the number of the data, respectively.
In our analysis, we consider the partial waves up to the $D$-wave ($l=2$).
We restrict the energy region up to $p_{\rm lab} = 800$ MeV/c, where the inelastic contribution
such as pion production starts to be significant.

\begin{table}[t]
\begin{center}
\caption{The determined parameters for the $I=1$ and $I=0$ amplitudes. There are two
parameter sets.
Solutions 1 and 2 are characteristic in reproduction of the experimental data. (See text in details.)
The values of the parameters $b^{I}, d^{I}, g^{I}$ and $h^{I}$ are shown in unit of $10^{-3}\ {\rm MeV}^{-1}$.
The subtraction constants for $I=0$ and $I=1$ are fixed as $a^{I=0, 1}=-1.150$.}
\begin{tabular}{c c| D{.}{.}{4}D{.}{.}{4} }
\hline
  & & \multicolumn{1}{c}{Solution 1}  & \multicolumn{1}{c}{Solution 2}  \\
 \hline  \hline
          &$b^{I=1}$         &0.54        &0.30        \\
          &$d^{I=1}$         &-0.29       &-0.24         \\
$I=1$  &$g^{I=1}$         &0.05       &0.72        \\
           &$h^{I=1}$         &0.03       &1.05       \\
           & $\chi^{2}/N$    &2.96       &2.97     \\
\hline
          &$b^{I=0}$         &0.11        &-0.46          \\
          &$d^{I=0}$         &0.33       &0.73       \\
$I=0$  &$g^{I=0}$         &-0.42       &0.56        \\
           &$h^{I=0}$         &1.14        &-3.54     \\
           & $\chi^{2}/N$    &4.54       &4.06     \\
\hline
\end{tabular}
\label{tab:parameter}
\end{center}
\end{table}

First of all, we determine the $I=1$ scattering amplitude from the $K^{+}p$
elastic scattering data, which were observed well with small
variation and certainly constrain the $I=1$ parameters.
To fix the $I=1$ low-energy constants $b^{I=1}, d^{I=1}, g^{I=1}$ and $h^{I=1}$,
we use the $K^{+}p$ differential cross section between
$p_{{\rm lab}} = 145$ to 726 MeV/c \cite{cameron1974}
and the total cross section between $p_{{\rm lab}} = 145$ to 788 MeV/c
\cite{bugg1968, bowen1970, adams1971,bowen1973, carroll1973, cameron1974}.
The fitted values of the parameters are summarized in the Table \ref{tab:parameter}.
We find two solutions for $I=1$, which equivalently reproduce the cross sections.
In Fig.~\ref{fig:i1_tot}, we present the total cross sections of the $I=1$ $KN$ elastic scattering
obtained with the fitted parameters and compare with the experimental
data~\cite{bugg1968, bowen1970, adams1971,bowen1973, carroll1973, cameron1974}.
The calculated amplitude gives a good reproduction of the data up to $p_{{\rm lab}}=$800~MeV/c.
It shows that the $S$-wave contribution is dominated
and the contributions from the partial waves higher than the $P$-wave are negligibly small.
This is consistent with the old observation.
In Fig.~\ref{fig:kp_diff}, we show the calculated differential cross sections
and make a comparison with the experimental data.
The figure shows that the obtained amplitudes reproduce the experimental data well
for all the energies which we consider here.

\begin{figure}[]
    \begin{tabular}{c}

      \begin{minipage}[t]{1.0\hsize}
        \centering
        \includegraphics[keepaspectratio, scale=0.8,bb=0 0 360 252]{tot1_sol1.pdf}

      \end{minipage} \\

      \begin{minipage}[t]{1.0\hsize}
        \centering
        \includegraphics[keepaspectratio, scale=0.8,bb=0 0 360 252]{tot1_sol2.pdf}

      \end{minipage} \\

    \end{tabular}
     \caption{The calculated $I=1$ total cross sections using Solutions 1 and 2 in comparison
with the experimental data \cite{bugg1968, bowen1970, adams1971,
bowen1973, carroll1973, cameron1974}.
  The partial wave components are also described by the dashed line.
  The horizontal axis means the $K^{+}$ meson incident momentum
  in the lab frame $p_{{\rm lab}}$ in the unit of MeV/c
  and the vertical axis is the total cross section $\sigma$ in the unit of mb.
}
\label{fig:i1_tot}
  \end{figure}

\begin{figure}[]
 \begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl145.pdf}
  \end{center}

 \end{minipage}
 \begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl175.pdf}
  \end{center}

 \end{minipage}
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl205.pdf}
  \end{center}

 \end{minipage}
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl235.pdf}
  \end{center}

 \end{minipage}
 \begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl265.pdf}
  \end{center}

 \end{minipage}
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl295.pdf}
  \end{center}

 \end{minipage}
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl325.pdf}
  \end{center}

 \end{minipage}
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl355.pdf}
  \end{center}

 \end{minipage}
 \end{figure}

 \begin{figure}[]
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl385.pdf}
  \end{center}

 \end{minipage}
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl500.pdf}
  \end{center}

 \end{minipage}

\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl613.pdf}
  \end{center}

 \end{minipage}
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl726.pdf}
  \end{center}

 \end{minipage}
 \vspace{-0.5cm}
\caption{
The calculated differential cross sections of the $K^{+}p$ elastic scattering
using Solutions 1 and 2
in comparison with the experimental data of Ref. \cite{cameron1974}.
}
\label{fig:kp_diff}
\end{figure}

Next, we determine the $I=0$ low-energy constants $b^{I=0}, d^{I=0}, g^{I=0}$ and $h^{I=0}$
using the data of the $K^{+}n \to K^{+}n$ and $K^{+}n \to K^{0} p$ differential cross sections
at $p_{{\rm lab}} = 526$, 604 and 640 MeV/c given in Refs \cite{Giacomelli:1972uj, Giacomelli:1973ed, dam1975}
together with  the $I=0$ total cross section of Ref.~\cite{bowen1970}
between $p_{{\rm lab}} = 366$ to 717 MeV/c,
which is referred as Bowen 1970 in Fig. \ref{fig:i0_tot}.
We have confirmed that even if we include the $I=0$ total cross section
of Ref. \cite{carroll1973} referred as Carroll 1973 in Fig. \ref{fig:i0_tot},
we obtain similar parameter sets with much worse $\chi^{2}$ values.
It would imply that our model prefers the data of Bowen 1970 \cite{bowen1970} and 1973 \cite{bowen1973}.
As a fine-tuning, we use the data of Bowen 1970 as the $I=0$ total cross section data.
The $K^{+}n$ elastic and charge exchange scattering amplitudes
are linear combinations of the $I=0$ and $I=1$ amplitudes
as shown in Eqs.~(\ref{eq:Kn}) and (\ref{eq:CE}).
The $I=1$ amplitude is already determined with the $K^{+}p$ elastic scattering.
The $I=1$ parameters are fixed, when the $I=0$ parameters are determined.
The fitted results for the $I=0$ parameters are summarized in the Table \ref{tab:parameter}.
Here we propose two solutions which have different character in the $I=0$ total cross section,
as we will discuss in details later.
In Fig.~\ref{fig:i0_tot}, we show the $I=0$ total cross sections calculated with Solution 1, 2 and
find that these two solutions reproduce well the observed total cross section.
The band
shown in the figure show the allowable region of each solution around the
vicinity of the local minimum of $\chi^{2}$, that is
$4.54<\chi^{2}/N<5.53$ for Solution 1
and  $4.06<\chi^{2}/N<5.01$ for Solution 2.
As one can see, the $I=0$ total cross section rapidly increases around $p_{\rm lab} = 500$ MeV/c.
In the two solutions, the partial wave which is responsible for the rapid increase of the cross section
is different.
Actually, as we shall see later, this feature links to the property of
a possible resonance appearing in $I=0$ with a large width.
In Solution 1, the $P_{01}$ amplitude\footnote{
We use the partial wave convention $L_{I\, 2J}$ with orbital angular momentum $L$,
isospin $I$ and total angular momentum $J = L \pm 1/2$.}
dominantly contributes, and thus
the rapid increases is caused by the $P_{01}$ amplitude. In Solution 2,
both $P_{01}$ and $P_{03}$ amplitudes provide the contribution for the $I=0$ total
cross section and the $P_{03}$ amplitude is responsible for the rapid increase.
In this way, these two solutions have
their own characteristic features in the $I=0$ total cross section.
In summary, we would say that Solution 1 is ``$P_{01}$ dominant solution",
Solution 2  is ``$P_{03}$ dominant solution".
In the following, we show the result of the differential cross sections used $I=0$ and 1 amplitudes.
Similar to the $I=0$ total cross section, we show the allowable region of solutions as the band.
Figures \ref{fig:kn_diff_sol1} and \ref{fig:kn_diff_sol2} show
the $K^{+}n$ elastic differential cross section for Solutions 1 and 2.
Solutions 1 and 2  are mostly consistent with the experimental data.
Figures \ref{fig:cex_diff_sol1} and \ref{fig:cex_diff_sol2} show the $K^{+}n$ charge exchange differential cross section.
Solutions 1 and 2 show relatively good reproduction except for the forward and backward scattering.
We cannot find sizable contradictions for Solutions 1 and 2 with the experimental data.
As seen later, other analyses support Solution 1.

\begin{figure}[]
    \begin{tabular}{c}

      \begin{minipage}[t]{1.0\hsize}
        \centering
        \includegraphics[keepaspectratio, scale=0.8, bb=0 0 360 252]{tot0_sol1.pdf}

      \end{minipage} \\

      \begin{minipage}[t]{1.0\hsize}
        \centering
        \includegraphics[keepaspectratio, scale=0.8,bb=0 0 360 252]{tot0_sol2.pdf}

      \end{minipage} \\

    \end{tabular}
     \caption{
   The $I=0$ total cross sections calculated using Solutions 1 and 2 in comparison
  with the experimental data \cite{bowen1970, bowen1973, carroll1973}.
  The solid line shows that the best-fit solution.
  The shaded area shows that the allowable region of the parameter around
  the vicinity of the best-fit solution.
  }
\label{fig:i0_tot}
  \end{figure}
\begin{figure}[]
 \begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm, bb=0 0 360 252]{pl434_kn.pdf}

  \end{center}

 \end{minipage}
 \begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm, bb=0 0 360 252]{pl526_kn.pdf}
  \end{center}

 \end{minipage}
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm, bb=0 0 360 252]{pl604_kn.pdf}
  \end{center}

 \end{minipage}
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm, bb=0 0 360 252]{pl640_kn.pdf}
  \end{center}

 \end{minipage}

 \begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm, bb=0 0 360 252]{pl688_kn.pdf}
  \end{center}

 \end{minipage}
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm, bb=0 0 360 252]{pl720_kn.pdf}
  \end{center}

 \end{minipage}
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm, bb=0 0 360 252]{pl771_kn.pdf}
  \end{center}

 \end{minipage}
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm, bb=0 0 360 252]{pl780_kn.pdf}
  \end{center}

 \end{minipage}
 \vspace{-0.5cm}
 \caption{
The differential cross sections of $K^{+}n$ elastic scattering
 using Solution 1
 in comparison with the experimental data of Ref. \cite{Giacomelli:1973ed, dam1975}.
The momenta at the $p_{{\rm lab}}$=640, 720 and 780 MeV/c are the data from Ref. \cite{Giacomelli:1973ed}.
The others are the data from Ref. \cite{dam1975}.}
\label{fig:kn_diff_sol1}
 \end{figure}
\begin{figure}[]
 \begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl434_kn2.pdf}
  \end{center}

 \end{minipage}
 \begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl526_kn2.pdf}
  \end{center}

 \end{minipage}
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl604_kn2.pdf}
  \end{center}

 \end{minipage}
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl640_kn2.pdf}
  \end{center}

 \end{minipage}

 \begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl688_kn2.pdf}
  \end{center}

 \end{minipage}
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl720_kn2.pdf}
  \end{center}

 \end{minipage}
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl771_kn2.pdf}
  \end{center}

 \end{minipage}
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl780_kn2.pdf}
  \end{center}

 \end{minipage}
 \vspace{-0.5cm}
 \caption{
The differential cross sections of $K^{+}n$ elastic scattering
 using Solution 2.}
\label{fig:kn_diff_sol2}
 \end{figure}

\begin{figure}[]
 \begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl434_n.pdf}
  \end{center}

 \end{minipage}
 \begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl526_n.pdf}
  \end{center}

 \end{minipage}
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl604_n.pdf}
  \end{center}

 \end{minipage}
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl640_n.pdf}
  \end{center}

 \end{minipage}

 \begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl688_n.pdf}
  \end{center}

 \end{minipage}
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl720_n.pdf}
  \end{center}

 \end{minipage}
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl771_n.pdf}
  \end{center}

 \end{minipage}
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl780_n.pdf}
  \end{center}

 \end{minipage}
 \vspace{-0.5cm}
 \caption{
 The differential cross sections of $K^{+}n$ charge exchange scattering
 using Solution 1 in
 comparison with the experimental data of Ref. \cite{Giacomelli:1972uj, dam1975}.
The momenta at the $p_{{\rm lab}}$=640, 720 and 780 MeV/c are the data from Ref.~\cite{Giacomelli:1972uj}.
The others are the data from Ref.~\cite{dam1975}. }
\label{fig:cex_diff_sol1}
 \end{figure}
\begin{figure}[]
 \begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl434_n2.pdf}
  \end{center}

 \end{minipage}
 \begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl526_n2.pdf}
  \end{center}

 \end{minipage}
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl604_n2.pdf}
  \end{center}

 \end{minipage}
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl640_n2.pdf}
  \end{center}

 \end{minipage}

 \begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl688_n2.pdf}
  \end{center}

 \end{minipage}
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl720_n2.pdf}
  \end{center}

 \end{minipage}
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl771_n2.pdf}
  \end{center}

 \end{minipage}
\begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{pl780_n2.pdf}
  \end{center}

 \end{minipage}
 \vspace{-0.5cm}
 \caption{
The differential cross sections of $K^{+}n$ charge exchange scattering
 using Solution~2.}
\label{fig:cex_diff_sol2}
 \end{figure}

\subsection{Possible broad resonances}
We have constructed the $KN$ amplitudes which reproduce the experimental data well.
In the following, we concentrate on the $KN$ partial wave amplitudes with $I=0$ and
discuss the outcome from the obtained amplitude.
First of all, we look for poles of the scattering amplitude in the complex energy plane.
Having the $KN$ scattering amplitude
in an analytic form, we can perform analytic continuation of the scattering amplitude into
the complex energy plane.
We find a pole in the $P_{01}$ amplitude of Solution 1 at $z = 1617 - 153 i$~MeV,
which corresponds to a resonance state with mass 1617~MeV/$\rm c^{2}$,
width 305~MeV and $J^{p} = (1/2)^{+}$.
The resonance has a quite large width and it could be hard to pin down the resonance
in production experiments.
Similarly, we find a pole of the $P_{03}$ amplitude of Solution 2 in the complex energy plane at
$z=1678 - 232 i $~MeV corresponding to a resonance state with mass
1678~MeV/${\rm c^{2}}$, width 463~MeV and $J^{p} = (3/2)^{+}$.
Since this resonance state
is located far from the real axis, it
is not constrained well by experimental observation
appearing in the real axis and theoretical uncertainty should be large and this solution
could be unstable against small deviation of experimental data.
These results are summarized in Table \ref{tab:amp}.
These resonances could be compared with the state found in the chiral soliton model \cite{weigel}
with around 1700 MeV/${\rm c^{2}}$ mass even though it has a narrow width.
In Fig. \ref{fig:poles}, we show the distribution of the poles in the vicinity of the best-fit value.

\begin{table}[]
\begin{center}
\caption{The resonance states of Solutions 1 and 2.}
  \begin{tabular}{l c c} \hline
    amplitude ($J^{P}$) & mass [MeV] &  width [MeV]  \\ \hline \hline
    Solution 1 \enspace $P_{01}$ ($ \frac{1}{2}^{+}$)  & 1617 & 305  \\ \hline
    Solution 2 \enspace $P_{03}$  ($ \frac{3}{2}^{+}$) & 1678  & 463  \\ \hline
  \end{tabular}
  \label{tab:amp}
  \end{center}
\end{table}

\begin{figure}[]
 \begin{center}

   \includegraphics[width=100mm,bb=0 0 3946 2705]{poles4.pdf}
 \end{center}
 \caption{The distribution of the poles of the amplitude in the complex energy plane $z$.
 The red star stands for the best-fit value.}
 \label{fig:poles}
\end{figure}

{Even though we find the resonance state as a pole of the scattering amplitude,
there are no peak structure in the scattering amplitude around the resonance energy.}
One usually expects
that resonance states should appear as a peak in the cross section. It is not necessarily true
when the resonance has a large width and substantial coupling to non-resonance background.
We demonstrate this situation by using a simple amplitude in which a resonance pole is embedded
in a constant background with a relative phase $\delta$:
\begin{equation}
  f(E) = \frac{i}{E - M + i \Gamma/2} + b e^{i\delta}. \label{eq:BWamp}
\end{equation}
In Fig.~\ref{fig:fano}, we show the cross sections of the amplitudes (\ref{eq:BWamp}) with
$\delta= 0, \frac{\pi}{2}, \pi, \frac{3\pi}{2}$ for $M=1600$ MeV, $\Gamma=300$ MeV and
$b=0.01$ MeV$^{-1}$.
As one can see in the figure, the resonance shape depends on the relative phase.
For $\delta=0$, the resonance and background contributions are interfered constructively
a resonance peak appears in the cross section, while for $\delta = \pi$, the resonance
and background contribute deconstructively and the resonance is seen as a dip.
It is very interesting to see that, for the case of $\delta=\pi/2$, a rapid increase
takes place at the resonance energy. This is also one of the resonance shapes.
These kinds of resonances are known as Fano resonance~\cite{Fano:1961zz}.
The resonance structure in the $KN$ $I=0$ channel might be one of
the example of Fano resonance.

\begin{figure}[]
 \begin{minipage}{0.24\hsize}
  \begin{center}
   \includegraphics[width=53mm,bb=0 0 360 252]{fano1_new.pdf}
  \end{center}

 \end{minipage}
 \begin{minipage}{0.24\hsize}
  \begin{center}
   \includegraphics[width=53mm,bb=0 0 360 252]{fano2_new.pdf}
  \end{center}

 \end{minipage}
  \begin{minipage}{0.24\hsize}
  \begin{center}
   \includegraphics[width=53mm,bb=0 0 360 252]{fano3_new.pdf}
  \end{center}

 \end{minipage}
   \begin{minipage}{0.24\hsize}
  \begin{center}
   \includegraphics[width=53mm,bb=0 0 360 252]{fano4_new.pdf}
  \end{center}

 \end{minipage}
\caption{Fano resonance. Cross sections of amplitudes composed of a resonance and
 a continuum background with relative phase $\delta$ are shown.
 The resonance is assumed to have 1600~MeV mass and 300 MeV width.
 The resonance shape is dependent on the relative phase $\delta$. The vertical axis is in arbitrary unit. }
\label{fig:fano}
\end{figure}

In Fig.~\ref{fig:amp_i0}, we show the real and imaginary parts of
the $I=0$ scattering amplitudes of $P_{01}$ for Solution 1 and
$P_{03}$ for Solution 2, where the resonances are found. As seen in figure,
a typical resonance structure is seen in the amplitudes, but the role of the real and imaginary
parts is interchanged. (Usually the imaginary part has a peak structure, while the real part
increases around the resonance point.) This is due to strong coupling of the resonance
to the continuum background with some relative phase. In order to confirm whether
the structure in the amplitude comes from the resonance state, we subtract
the resonance contribution from the amplitude.  We express the resonance contribution
as the Breit-Wigner form, of which the numerator is obtained
by calculating the residue of the amplitude at the resonance pole.
The subtracted amplitudes are shown as dotted lines in Fig,~\ref{fig:amp_i0}.
It implies that the subtracted amplitudes are almost constant without significant structure.
Thus, the structure appearing in the amplitudes is caused by the resonance state.

As we have mentioned above, the imaginary part of the amplitude rapidly
increases around the resonance energy. According to the optical theorem,
the total cross section is proportional to the imaginary part. Therefore,
we conclude that the rapid increase seen in the $I=0$ total cross section around
$p_{\rm lab}=500$ MeV/c can be a sign of the possible existence of a
resonance with a large width. In addition, the spin-parity of the resonance
can be learned by knowing which partial wave is responsible for the rapid increase
of the $I=0$ total cross section.
Here we have proposed
two solutions; in Solution 1, the rapid increase appears in the $P_{01}$-wave
and the resonance should have $J^{p} = (1/2)^{+}$. In Solution 2, it does
in the $P_{03}$-wave and the resonance should have $J^{p} = (3/2)^{+}$.
It would be very interesting if one could understand the feature of the
$I=0$ total cross section around $p_{\rm lab}=500$ MeV/c with more accurate
experimental data.

\begin{figure}[]
    \begin{tabular}{c}

      \begin{minipage}[t]{1.0\hsize}
        \centering
        \includegraphics[keepaspectratio, scale=0.8,bb=0 0 360 252]{sol1_p01.pdf}

      \end{minipage} \\

      \begin{minipage}[t]{1.0\hsize}
        \centering
        \includegraphics[keepaspectratio, scale=0.8,bb=0 0 360 252]{sol2_p03.pdf}

      \end{minipage} \\

    \end{tabular}
     \caption{
     The real and imaginary parts of the $I=0$ amplitudes of $P_{01}$ for Solution 1,
     $P_{03}$ for Solution 2 around the resonance energy.
     The solid lines stand for the original amplitudes, while
     the dotted lines stand for the amplitudes obtained by subtracting the resonance pole.}
\label{fig:amp_i0}
  \end{figure}

\begin{figure}[t]
 \begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{S01_SOL1.pdf}
  \end{center}

 \end{minipage}
 \begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{S01_SOL2.pdf}
  \end{center}

 \end{minipage}
 \begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{P01_SOL1.pdf}
  \end{center}

 \end{minipage}
 \begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{P01_SOL2.pdf}
  \end{center}

 \end{minipage}
   \begin{minipage}{0.50\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{P03_SOL1.pdf}
  \end{center}

 \end{minipage}
 \begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{P03_SOL2.pdf}
  \end{center}

 \end{minipage}
  \vspace{-0.5cm}
 \caption{The Argand diagrams of Solutions 1 and 2 in the $I=0$ states up to the momentum $p_{{\rm lab}}=$800 MeV/c.
 Solution 1 is compared with the Martin's amplitude \cite{martin1975} and SAID amplitude
  \cite{said} shown in the dotted line. It shows that Solution 1 is consistent with existing partial wave amplitude.}
\label{fig:arg_iso0}
 \end{figure}

In Fig. \ref{fig:arg_iso0},
we show the Argand diagrams of the $I=0$ scattering amplitudes for the $S$ and $P$-wave
up to $p_{{\rm lab}}=$ 800 MeV/c using Solutions 1 and 2.
Then we compare with Martin's amplitude~\cite{martin1975} and amplitude of
SAID program~\cite{said}.
We find that the partial wave amplitudes for Solution 1 are very similar to the Martin's amplitude
and amplitude of SAID program.
Thus, one could find a pole for a board resonance also in the Martin's amplitude
and amplitude of SAID program.
It is also interesting to point out that, for Solution 2, the $P_{03}$ channel has an attraction
interaction and actually hold a broad resonance, while the $P_{01}$ channel is repulsive
even though some contribution of $P_{01}$ is seen in the total cross section.
In~Fig.~\ref{fig:energy_amp}, we show the momentum dependence of the $I=0$ partial-wave
$T$-matrix~$T^{\prime}_{l \pm}$ defined by $T^{\prime}_{l \pm} = -kT_{l \pm}/(8\pi\sqrt{s})$,
where  $T_{l \pm}$ is given
in Eq.~(\ref{eq:less_amp}), for Solutions~1 and 2 in comparison with Martin's amplitude~\cite{martin1975} and SAID amplitude~\cite{said}.
The solid and dashed lines stand for the real and imaginary parts of the amplitudes, respectively.

\begin{figure}[t]
 \begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{amp1_S01.pdf}
  \end{center}

 \end{minipage}
 \begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{amp2_S01.pdf}
  \end{center}

 \end{minipage}
 \begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{amp1_P01.pdf}
  \end{center}

 \end{minipage}
 \begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{amp2_P01.pdf}
  \end{center}

 \end{minipage}
   \begin{minipage}{0.50\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{amp1_P03.pdf}
  \end{center}

 \end{minipage}
 \begin{minipage}{0.5\hsize}
  \begin{center}
   \includegraphics[width=80mm,bb=0 0 360 252]{amp2_P03.pdf}
  \end{center}

 \end{minipage}
  \vspace{-0.5cm}
 \caption{
 The dimensionless partial-wave amplitudes $T^{\prime}_{l \pm} = -kT_{l \pm}/(8\pi\sqrt{s})$
 of Solutions 1 and 2 in the $I=0$ channel up to the momentum $p_{{\rm lab}}=$800~MeV/c
 in comparison with Martin's~\cite{martin1975} and SAID~\cite{said} amplitudes.
 The solid and dashed lines stand for the real and imaginary parts of the amplitudes, respectively.}
\label{fig:energy_amp}
 \end{figure}

It would be interesting to show a theoretical amplitude
which was the rapid increase of the $I=0$ total cross section in $S$-wave.
We find such a solution with the parameter set called Solution 3 given in Table \ref{tab:sol3}.
Figure \ref{fig:tot3} shows the $I=0$ total cross section.
It shows that the $S_{01}$ amplitude substantially contributes and
the rapid increase of the cross section stems from the $S_{01}$ amplitude.
Solution 3 cannot reproduce the angular dependence of the differential cross section
of the charge exchange, because the amplitude of Solution 3 is composed of $S$-wave contribution.
Thus, Solution 3 could be ruled out.
Nevertheless, here we discuss also Solution 3, because we want to point out
the relation between the rapid increase of the $I=0$ total cross section and existence of the
possible broad resonance.
We find a pole in the $S_{01}$ amplitude of Solution 3 at $z = 1624 - 132i$ MeV,
which corresponds to a resonance state with 1624 MeV/${\rm c^{2}}$, width 264 MeV and $J^{P}=(1/2)^{-}$.
In Fig. \ref{fig:amp3}, we show the real and imaginary part of the $S_{01}$ amplitude
for Solution 3 and find the resonance structure in the amplitude.

\begin{table}[]
\begin{center}
\caption{
The $S$-wave parameter set.
}
\begin{tabular}{c c| D{.}{.}{4}}
\hline
           &                      & {\rm Solution 3} \\
 \hline  \hline
          &$b^{I=1}$         &0.30     \\
          &$d^{I=1}$         &-0.24     \\
$I=1$  &$g^{I=1}$        &0.72   \\
           &$h^{I=1}$         &1.05  \\
           & $\chi^{2}/N$   &4.06\\
\hline
          &$b^{I=0}$        &0.38     \\
          &$d^{I=0}$       &0.01  \\
$I=0$  &$g^{I=0}$      &-1.35   \\
           &$h^{I=0}$        &-0.11  \\
           & $\chi^{2}/N$   &29.7\\
\hline
\end{tabular}
\label{tab:sol3}
\end{center}
\end{table}

\begin{figure}[]
 \begin{center}
  \includegraphics[width=100mm,bb=0 0 360 252]{tot0_sol3.pdf}
 \end{center}
 \caption{The $I=0$ total cross section calculated using the Solution 3.}
 \label{fig:tot3}
\end{figure}

\begin{figure}[]
 \begin{center}
  \includegraphics[width=100mm,bb=0 0 360 252]{sol3_s01.pdf}
 \end{center}
 \caption{The real and imaginary parts of the $S_{01}$ amplitude calculated using Solution 3.}
 \label{fig:amp3}
\end{figure}

\section{Conclusion}
\label{sec:sec4}
We have investigated the $KN$ elastic scattering below the energy where the
inelastic contributions become signifiant, that is, $p_{\rm lab} < 800$ MeV/c,
by describing the scattering amplitude in the chiral unitary approach as an analytic function.
We utilize a next-to-leading
chiral Lagrangian for the kernel interaction of the unitarized amplitude, and the
low energy constants in the  amplitude are determined to reproduce
the differential cross sections of $K^{+}p \to K^{+}p$, $K^{+}n \to K^{+}n$, $K^{+}n \to K^{0} p$
and the $I=0, 1$ total cross sections.
We have obtained good scattering amplitudes which reproduce the observed
scattering cross section very well. Particularly, the $I=1$ scattering amplitude,
namely $K^{+}p$ elastic amplitude, has been determined well thanks to less ambiguous
experimental data with small errors, and we have found that the $I=1$ scattering
amplitude at $p_{\rm lab}<800$ MeV/c is essentially described by
$S$-wave contribution, which is consistent with our conventional knowledge.
For the $I=0$ amplitude, we have proposed two possible parameter sets,
which reproduce the $I=0$ scattering cross sections similarly and have different
nature for the rapid increase appearing in the $I=0$ total cross section around
$p_{\rm lab} = 500$ MeV/c. In Solution 1, the rapid increase appears in $P_{01}$-wave
contribution,  while in Solution 2 it stems from the $P_{03}$-wave contribution.
To show the example of the rapid increase of the $I=0$ total cross section
in the $S_{01}$ amplitude by Solution 3,  even though it is not a realistic solution.

Having performed analytic continuation of the obtained $I=0$ scattering amplitudes
to the complex energy plane, we have found a pole corresponding to a broad resonance
state around
$E_{\rm c.m.} = 1617~{\rm MeV}$ with 305 MeV width in each scattering amplitude.
We would like to emphasize strongly that the existence of a broad resonance
is responsible for the rapid increase of the $I=0$ total cross section around $p_{\rm lab} =
500$ MeV/c. Thus, further investigation of the nature of the rapid increase
of the $I=0$ total cross section reveals directly the existence of the $S=+1$ exotic resonance
state. Usually resonance states, especially narrow resonances, appear as a bump
in the total cross section. Nevertheless, for broad resonances, because they strongly
couple to the non-resonance background, their resonance shape seen in the cross section
can be modified. This is known as Fano resonance.

In order to pin down the existence of the $S=+1$ broad resonance, one needs further
detailed investigation. First of all, the resonance found in this work has a broad width
and is located far from the real axis in the complex energy plane. The experimental
informations are in the real axis and constrain the scattering amplitude well close to the real axis.
To make the scattering amplitude, or the position of the pole, constrained more,
more accurate experimental data are necessary. In addition, one also needs more reliable
theoretical description. For instance, it could be necessary to introduce more terms
into the interaction kernel. It is also important to describe $K^{+}d$ scattering with
the deuteron wavefunction theoretically. This makes us to perform direct comparison
of the theoretical calculation to the experimental observation.

\section*{Acknowledgment}

The authors would like to thank Dr.\ T.~Hyodo for his helpful comments.
The work of D.J.\ was partly supported by Grants-in-Aid for Scientific Research from JSPS (17K05449).

redpajama_set_name: RedPajamaArXiv


Truly a night to remember fondly, for grads, and parents.
We wish to wholeheartedly thank Darlene Younger and her amazing crew of volunteer organizers for a phenomenal 2012 Belmont secondary school prom. By all accounts, the dinner was great, the photo booth and dance a lot of fun, and the 'Enchanted Forest' theme was, well, enchanting.
Also, we would like to thank Principal Carl Repp and his dedicated admin team, for organizing an outstanding dry grad, giving our kids a choice for a more wholesome evening of celebration, which included bowling, mini golf, laser tag, rock climbing, a mechanical bull, breakfast and prizes for all.
Last, but certainly not least, we would like to thank all of the parent volunteers who helped make both events happen.


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Northern Ireland Protocol
Government urged to 'adopt own state aid system'
The UK government should look to create its own state aid system after the Brexit transitional agreement ends, according to the Institute for Government.
£355m announced for Northern Ireland goods system
The government is set to spend £335m on a new system for moving goods into Northern Ireland from the rest of the UK.


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Taking Alarm: The Importance of the International Religious Liberty Association
Posted by ReligiousLiberty.TV	/ April 16, 2012
Next week the 7th World Congress of the International Religious Liberty Association (IRLA) will be taking place in the Dominican Republic. The IRLA has been in operation since 1893, making it one of the oldest associations that is dedicated to freedom of conscience.
The theme of the conference is "Secularism and Religious Freedom-Conflict or Partnership?" which will differentiate between secularism in terms of separation of church and state under which faith can freely thrive and hostile radical secularism which seeks to marginalize religion. Other topics up for discussion will include the impact of the recent government changes in Egypt, Libya, and Syria.
Since 2003, the United Nations has recognized the IRLA as a Category II Non-Governmental Organization and its thirteen regions cover the globe. Although this organization, comprised of a volunteer staff, was started by the Seventh-day Adventist Church, it is non-sectarian and many other religious traditions who value liberty of conscience are involved in its operation.
In February 24, 1893, the General Conference of Seventh-day Adventists meeting in Battle Creek, Michigan adopted a Resolution and Remonstrance objecting to a U.S. Supreme Court decision that had essentially declared the United States a "Christian nation" when deciding that the World's Fair should close on Sundays. The argument the Court made in supporting its decision, more than the issue of Sunday itself, was the subject of the objection.
The Supreme Court had stated that, "There is no dissonance in these declarations. There is a universal language pervading them all, having one meaning. They affirm and reaffirm that this is a religious nation. These are not individual sayings, declarations of private persons. They are organic utterances. They speak the voice of the entire people. While because of a general recognition of this truth the question has seldom been presented to the courts, yet we find that in Updegraph v. Com., 11 Serg. & R. 394, 400, it was decided that, �Christianity, general Christianity, is, and always has been, a part of the common law of Pennsylvania."- Supreme Court Decision, 1892 Church of the Holy Trinity Decision v United States.
In response, the Adventist Church objected to the assertion that the government could define religion, and stated that "religion, or the duty which we owe to our Creator, and the manner of discharging it, can be directed only by reason and conviction, and is nowhere cognizable but at the tribunal of the universal Judge."
Describing the decision, the resolution drafted by A.T. Jones stated, "It is proper to take alarm at the first experiment on our liberties. We hold this prudent jealousy to be the first duty of citizens and the noblest characteristic of the American Revolution. The freemen of America did not wait till usurped power had strengthened itself by exercise and entangled the question in precedents. They saw all the consequences in the principle, and avoided the consequences by denying the principles."
In arguments that are remarkably pertinent to the issues we face in 2012, the resolution states, "We, therefore, as Christians, as Protestants, as American citizens, and as men, appealing to the Supreme Judge of the world for the rectitude of our intentions, do, in the name and by the authority of the natural rights of mankind, of the Constitution of the United States, of history of more than eighteen hundred years, and of the Lord Jesus Christ, solemnly publish and declare that we are and of right ought to be, free and independent of all connection, direction, dictation, interference, or control, of the government of the United States, in matters of religion or religious observances or religious institutions of any kind or degree; and that, as such, so far as earthly authority is concerned, we have full right to be religious or not religious, to worship or not to worship, to observe a day or not to observe it, according to the dictates of our own consciences and the convictions of our own minds."
The full document as well as additional materials including the Supreme Court decision in Church of the Holy Trinity v. United States, 143 U.S. 457 (1892) is available at the Adventist Archives.
The IRLA has adopted the following set of principles:
We believe that religious liberty is a God-given right.
We believe that legislation and other governmental acts which unite church and state are contrary to the best interests of both institutions and are potentially prejudicial to human rights, and hold that it is best exercised where separation is maintained between church and state.
We believe that government is divinely ordained to support and protect citizens in their employment of natural rights, and to rule in civil affairs; and that in so doing, government warrants respectful obedience and willing support.
We believe in the natural and inalienable right of freedom of conscience – to have or not to have a religion; to adopt the religion or belief of one's choice; to change religious belief according to conscience; to manifest one's religion individually or in community with others, in worship, observance, practice, promulgation and teaching – subject only to respect for the equivalent rights of others.
We believe that religious liberty includes also the freedom to establish and operate appropriate charitable or educational institutions, to solicit or receive voluntary financial contributions, to observe days of rest and celebrate holidays in accordance with the precepts of one's religion, and to maintain communication with fellow believers at national and international levels.
We believe that religious liberty and the elimination of intolerance and discrimination based on religion or belief are essential to promote understanding, peace and friendship among people.
We believe that citizens should use lawful and honorable means to prevent the reduction of religious liberty, so that all may enjoy its inestimable blessing.
We believe that the spirit of true religious liberty is epitomized in the Golden Rule: Do unto others as you would have others do unto you.
Today, the International Religious Liberty Association continues forward with a global focus on freedom. While many religious organizations address religious freedom from the perspective of one nation or another, the IRLA recognizes that what one nation does may affect the liberty of people in other nations, and so efforts are designed to coordinate between people of faith in various countries.
Much of this international focus is probably due to the fact that the Seventh-day Adventist Hospital operates, under a single umbrella, churches, hospitals, schools, and colleges and a variety of other institutions around the world. If freedom is curtailed in one place, the impact is acutely felt elsewhere.
News and video updates of the IRLA Conference are going to be made available at http://www.irla.org.
It is wonderful how much time good people spend fighting the devil. If they would only expend the same amount of energy loving their fellow men, the devil would die in his own tracks of ennui.
— Helen Keller
Blessed are the Peacemakers: Why Adventist Clergy Stay Away from Partisan Politics
Lautenberg Act, Created to Give Religious Immigrants a Fast Pass, in Jeopardy
Home » Taking Alarm: The Importance of the International Religious Liberty Association


Welcome to the Microsoft Payments Community.
In this blog, I will share my thoughts and insights into the payments industry, and the challenges banks face in renewing their core platforms.
Many people ask me, "why the interest in payments systems?" Quite honestly, it's an easy answer: payments make the world go around. In mature and emerging economies, every business transaction results in a transfer of value, or a payment, somewhere.
To meet these challenges requires a strategic response. Microsoft payments solution areas, delivered through our community of partners, are well suited to address each of these challenges, and so I encourage you to read more about how we can be of benefit to your business.


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Medway Secure Training Centre judged 'Inadequate' by Ofsted
A recent Ofsted report has judged Medway Secure Training Centre (MSTC) to be 'Inadequate', the lowest score awarded by Ofsted.
The Centre, a young offenders institute In Evelyn Road, Rochester, was found to be putting children at risk of harm despite a serious case review following the BBC Panorama in 2016.
MSTC will close in Spring 2020 and be reopened as the country's first Secure School.
I'm seriously concerned about the government's decision to turn MSTC, an institution beset by systemic failures over the last few years, into the country's first Secure School. Cllr Clive Johnson, Medway Labour Shadow Cabinet Member for Children and Young People
Cllr Clive Johnson, Medway Labour Shadow Cabinet Member for Children and Young People said, 'It is completely unacceptable that very little has changed at Medway Secure Training Centre, despite three Ofsted inspections since 2017.
'Ofsted has found that children are still "at risk of harm" and are even being denied hospital treatment.
'I'm seriously concerned about the government's decision to turn MSTC, an institution beset by systemic failures over the last few years, into the country's first Secure School.
'By commissioning Oasis Charitable Trust – an organisation which appears to lack any experience in looking after children in a residential setting – to run the new Secure School, the government is setting itself up to repeat the same mistake it made by giving G4S the contract to run MSTC.
'If the government is serious about ensuring the new Secure School will help rehabilitate and reintegrate these children back into society, then they need to learn from their mistakes and commit to treating these children with dignity and respect.'
Sadly, the empty rhetoric on crime we have heard from Home Office ministers recently suggests none of those lessons have been learned. It will give me no satisfaction if, as a result, history repeats itself in Medway under the new provider Cllr Alex Paterson, Medway Labour & Co-operative Councillor for Rochester West
Cllr Alex Paterson, Medway Labour & Co-operative Councillor for Rochester West said 'It's estimated that it's five times more expensive to lock up young offenders than it would be to send them to Eton.
'The great irony is that in my experience of meeting young offenders in Rochester, many of them have the clear potential to lead productive, fulfilled and law-abiding lives given the opportunity.
'However as a society we are complicit in a system which often merely brutalises vulnerable young people, entrenches those behaviours which got them into trouble in the first place and prepares them for a life of crime.
'That is not only a waste of taxpayers' money, it is a waste of human lives and does nothing to make our streets any safer.
'Sadly, the empty rhetoric on crime we have heard from Home Office ministers recently suggests none of those lessons have been learned. It will give me no satisfaction if, as a result, history repeats itself in Medway under the new provider.'
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Generally cloudy. A few flurries or snow showers possible. High 26F. Winds W at 10 to 20 mph..
West Virginia guard Tynice Martin (5) during the second half of an NCAA college basketball game against Mississippi State, Sunday, Dec. 8, 2019, in Starkville, Miss. (AP Photo/Vasha Hunt)
Vasha Hunt
West Virginia looks to continue winning ways against Texas
By Bob Hertzel For the Times West Virginian
MORGANTOWN — On Friday, Baylor's women's basketball team stunned No. 1 Connecticut and ended their 98-game home winning streak with a convincing 74-58 victory — the repercussions of the Bears victory were felt all the way to Morgantown.
It was not only a statement game for Bayor, but also for the entire Big 12. That is really important for Mike Carey's West Virginia team, who is carving out its own niche in the Big 12 and may well be the only thing standing between the Bears and a conference title.
But first, of course, this young and growing Mountaineer has to take care of its own business and that means finding a way to defeat a tough Texas team as it returns to the Coliseum at 1 p.m. for its Big 12 home opener.
This is something less than a statement game for WVU — which stands at 12-1 and holds a No. 20/19 ranking, — but if they are to get to the point where they are playing statement games they need to be a 7-5 Texas team.
"It's early," Coach Mike Carey admitted when asked if this meeting could qualify as a statement game for a team that has failed to reach the NCAA's the past two years. "Even if we win it, it's not like 'Oh, boy, we're here.' If we lose it we're not out of anything. It's an important game. It's at home. We need to take care of home court. You need to take win your home games and split on the road. You do that and you're fine."
Veteran Tynice Martin understands the importance of the game.
"Every game is like that for us. We take it kind of personal. We get up every game. Coach Carey fires us up. No matter how many wins we have, he kind of lets us know that we have to stay humble. We haven't gotten there yet," the senior said.
"The last two years we've been in the NIT and he's making sure we don't go down that road again. This is a big game just like every other game."
And the freshmen like KK Deans get it, too.
"This is a big game," she said. "We're going to be ready. We'll fight. if everyone does their part and plays their role, we'll have the same outcome we've been having."
Carey believes he has the makings of a team that can compete this year, despite its youth.
"There's times we played very well. There's games we played very well, and there were games when we didn't. We're still inconsistent. Our inside game needs to get a lot better. We're not getting a lot of scoring from that right now," he said.
"We have to take some pressure off our guards becaue they are overloading on that because we're not scoring inside. We have to keep getting better. The season is early and we have a lot of tough games coming up. We'll see where we're at against Texas."
Texas is a team that relies on two big inside players and that plays a physical game, winning five of its last six games.
"I've been watching tape and they are playing better. They are playing with more energy. The Higgs girl is playing better now that she has gotten used to playing again. She sat our last year," Carey said, referring to second team All-Big 12 player Lashann Higgs, who played four games last season before ending it with knee surgery.
"They are a good team. They are very big, very strong, physical. They have athletes out on the perimeter. We are going to have to defend them. What makes them tougher is the 4 and 5 will pop out for 3s. We have to defend that."
Follow Bob Hertzel on Twitter @bhertzel
Lashann Higgs


Thanks to its multi-functional structure, Sinerga is able to offer a "full service" approach for the development of cosmetics, dermo-pharmaceuticals and medical devices.
The extensive experience in the pharmaceutical and dermo-cosmetic fields and the continuous updates on regulatory field, market trends and scientific innovations make Sinerga a real reference point in this sector and a capable partner to create successful products.
Product Design according to customer's brief and/or following our suggestions.
Technical and marketing support for the right market positioning.
Management of performance and clinical tests.
Regulatory assistance, drafting P.I.F. and technical files.
Quality controls and quality assurance.
Technical and marketing support for the product launch.
A selected Project Manager in R&D Lab takes care of the whole project and becomes the customer's reference throughout the development process and the product finalization.
Sinerga's "full service" stands out for proactivity, experience, reliability, excellent problem solving and focus on customers' needs.
A single contact to interface with, who is aware of the project's progresses.
Time Optimization: the "time to market" is speeded by removing the intermediate steps with external agents.
A direct interaction among the company's departments involved in the product development for a greater flexibility and promptness in response.
A specific Know-how focused on the field.


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La Ligue A 2021-2022, 81ª edizione della massima serie del campionato francese di pallavolo femminile, si è svolta dall'8 ottobre 2021 al 7 maggio 2022: al torneo hanno partecipato quattordici squadre di club francesi e la vittoria finale è andata per la prima volta al .

Regolamento

Formula
La formula ha previsto:
 Regular season, disputata con girone all'italiana, con gare di andata e ritorno, per un totale di ventisei giornate (l' non ha concorso ai fini della classifica finale): le prime otto classificate hanno acceduto ai play-off scudetto, mentre l'ultima classificata è retrocessa in Élite.
 Play-off scudetto, disputati con:
 Quarti di finale e semifinali, giocate al meglio di due vittorie su tre gare.
 Finale, giocata al meglio di tre vittorie su cinque gare.

Criteri di classifica
Se il risultato finale è stato di 3-0 o 3-1 sono stati assegnati 3 punti alla squadra vincente e 0 a quella sconfitta, se il risultato finale è stato di 3-2 sono stati assegnati 2 punti alla squadra vincente e 1 a quella sconfitta.

L'ordine del posizionamento in classifica è stato definito in base a:
Punti;
Numero di partite vinte;
Ratio dei set vinti/persi;
Ratio dei punti realizzati/subiti.

Squadre partecipanti

Torneo

Regular season

Risultati

Classifica

Legenda:
      Qualificata ai play-off scudetto.
      Retrocessa in Élite.

Play-off scudetto

Tabellone

Risultati

Quarti di finale

Semifinali

Finale

Verdetti

Statistiche

Note

Collegamenti esterni

Pallavolo nel 2021
Pallavolo nel 2022
 2021-2022


Why a Humanitarian Award Means a Lot?
There are all kinds of awards given to different people for different reasons. While most of the awards are usually awarded for some kind of a competitive achievement there are special awards given to people who have done something remarkable to help others. Humanitarian awards are one such group of awards. These awards are given to people who have helped for the welfare of human beings. Even governments offer these kinds of awards.
If you look at a notable entrepreneur such as Teo Yen Koon Desmond you will see that he has been awarded the US President Lifetime Achievement Award for the community service he has done. It is not something given to everyone. You have to be truly involved in a huge amount of community service to be admired in that way. A humanitarian award carries a lot of value because it is important in a couple of different ways.
Getting a humanitarian award is not an easy task. We think getting an award for academic achievements is hard. However, that only requires you to use your intellect and write answers. With a humanitarian award you have to truly dedicate your life to make the lives of others better. It is not an easy task.
A humanitarian award is only offered to those who have actually done great service to the community they live in. This can be a project such as getting clean water to an area where people suffer from lack of fresh and clean water. All of these humanitarian projects for which humanitarian awards are given are not easy at all.
The only people who succeed in getting a humanitarian award are those who are really passionate about helping other people. You cannot face the problems and the pressure you will meet along the way of helping others if you are not truly passionate about helping others. So, only people with a real passion to help others are the ones who get such a humanitarian award.
Getting such an award may be sometimes less important than the love and respect one gets from people. Still having such a humanitarian award can help the person to get more help from people with the ability to help in the future.
These reasons make a humanitarian award very important. There is a lot you can achieve with the help of such a humanitarian award if you are into community service.


World Cup Scrapbook: "We're on the bus!"
Since the walk back to downtown Nuremberg seemed a bit daunting following the Fanfest, we crowded aboard a bus jam packed with jubilant England fans. Upon boarding, this group quickly turned the tune of "Football's Coming Home" into "We're on the bus, we're on the bus, we're on the, we're all on the bus!" I don't think the guy in the orange hat was amused.