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El Jardines y Parque del Guadalupe River (en inglés: Guadalupe River Park & Gardens, es un jardín botánico y parque ciudadano de 1.5 km² de extensión, administrado por la sociedad « Friends of Guadalupe River Park & Gardens, » en colaboración con el ayuntamiento de San José, California, Estados Unidos.

Localización
El jardín botánico se ubica en San José.

Guadalupe River Park & Gardens, 438 Coleman Avenue, San José, Santa Clara county, California CA 95110-2004 United States of America-Estados Unidos de América.

Planos y vistas satelitales.

La entrada es gratuita.

Historia
Los jardines de Guadalupe están localizados al sur del aeropuerto internacional de Mineta San José (y adyacente al parque del río) donde las casas fueron quitadas debido al ruido de hace unos 20 años.

El plan maestro para esta área fue desarrollado por la ciudad de San José y un grupo de trabajo de ciudadanos. La tierra vacía que compone gran parte de esta zona, será transformada en toda una serie de jardines para el goce público.

Colecciones
Este jardín botánico alberga varias secciones temáticas,

 Courtyard Garden and Taylor Street Rock Garden (Jardín del Patio y Rocalla de la Calle Taylor), estos fueron los primeros elementos de los jardines de Guadalupe que se terminaron. Una gama de plantas flor, con hierba de césped, y arbustos se ofrecen en el jardín del patio. La rocalla tiene lo último en ajardinamiento tolerante de la sequía. En 1999, después de que el sistema de riego fuera conectado al agua reciclada, la asociación de los amigos del parque del río de Guadalupe impulsó la creación de este jardín. El propósito del jardín es la demostración para los profesionales del paisaje y al público en general cómo unas variedades de plantas reaccionan al agua reciclada en un paisaje de diseño.
 Heritage Rose Garden (Rosaleda de la Herencia), es una rosaleda que alberga una colección de 3,700 rosas tanto antiguas como modernas. Creado en 1995 gracias a un esfuerzo de la comunidad.
 Historic Orchard (Huerto histórico), es un huerto de 3.3 acres plantado en 1994 para mostrar las variedades de árboles frutales que una vez hicieron famoso el valle de Santa Clara como "The Valley of Heart's Delight". Está situado en los jardines de Guadalupe al sur de "Taylor Street" y adyacente al parque del río. La huerta contiene unos 250 árboles frutales, incluyendo cerezos, albaricoques, parras, manzanas, y más. Está mantenida por equipos de voluntarios.
 Columbus Park, ocupa el terreno de un antiguo barrio trasladado a otro lugar para dejar espacio como zona de aproximación del aeropuerto adyacente.

Enlaces externos
 Página oficial del Guadalupe River Park & Gardens
 Página del jardín botánico en el BGCI

Guadalupe river
Guadalupe river
Guadalupe river
Flora de California


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redpajama_set_name: RedPajamaCommonCrawl


text:
Eamonn Toland
Éamonn Toland read Modern History and Economics at St. Hugh's College, Oxford. He is the author of the forthcoming book, The Pursuit of Kindness, From Collaboration to Cruelty and Back Again: An Evolutionary History of Human Nature. He can be reached on Twitter @eamonntoland.
Brexiteers are the not the only Cakeists in town…
Eamonn Toland on December 1, 2022, 2:13 pm | Readers 4899
Forget Citizen's Assemblies, productivity gaps, and subventions. The real litmus test for Irish reunification has to involve more than a technocratic plan. It has to include a vision for how a new Ireland will "unite all the people who share the territory of the island of Ireland, in all the diversity of their identities and traditions". Copyright on Amhrán na bhFiann lapsed in 2012, which allowed Dunnes Stores, among others, to start printing the lyrics on t-shirts. Kathy Sheridan, in …
Would all nationalists vote for a new Ireland?
Eamonn Toland on March 30, 2020, 2:15 pm | Readers 4123
As discussion of a border poll has risen within the wider nationalist community, the debate about what would be needed to accommodate all identities in a new Ireland has barely begun. Ian Clarke's thoughtful piece on Slugger about whether pro union voices were wanted threw the lack of engagement between nationalists and unionists into sharp relief. In a largely nationalist milieu, it's easy to see how a new Ireland would look much like the current republic, but what if the proposals from …


—You, Cochrane, what city sent for him?
—There was a battle, sir.
The boy's blank face asked the blank window.
masonry, and time one livid final flame. What's left us then?
—I forget the place, sir. 279 B. C.
—Yes, sir. And he said: Another victory like that and we are done for.
leaned upon his spear. Any general to any officers. They lend ear.
—You, Armstrong, Stephen said. What was the end of Pyrrhus?
—I know, sir. Ask me, sir, Comyn said.
—Wait. You, Armstrong. Do you know anything about Pyrrhus?
proud that their eldest son was in the navy. Vico Road, Dalkey.
—Pyrrhus, sir? Pyrrhus, a pier.
more loudly, aware of my lack of rule and of the fees their papas pay.
whispered. Yes. They knew: had never learned nor ever been innocent.
—Kingstown pier, Stephen said. Yes, a disappointed bridge.
The words troubled their gaze.
—How, sir? Comyn asked. A bridge is across a river.
too often heard, their land a pawnshop.
that they never were? Or was that only possible which came to pass?
Weave, weaver of the wind.
—Tell us a story, sir.
—O, do, sir. A ghoststory.
—Where do you begin in this? Stephen asked, opening another book.
—Weep no more, Comyn said.
—After, Stephen said. Go on, Talbot.
It must be a movement then, an actuality of the possible as possible.
—Turn over, Stephen said quietly. I don't see anything.
—What, sir? Talbot asked simply, bending forward.
 Riddle me, riddle me, randy ro.
 My father gave me seeds to sow.
Talbot slid his closed book into his satchel.
—Have I heard all? Stephen asked.
—Yes, sir. Hockey at ten, sir.
—Who can answer a riddle? Stephen asked.
They bundled their books away, pencils clacking, pages rustling.
—A riddle, sir? Ask me, sir.
—Again, sir. We didn't hear.
—What is it, sir? We give it up.
—The fox burying his grandmother under a hollybush.
clamour of their boots and tongues.
and damp as a snail's bed.
He held out his copybook. The word Sums was written on the headline.
blind loops and a blot. Cyril Sargent: his name and seal.
Stephen touched the edges of the book. Futility.
—Do you understand how to do them now? he asked.
copy them off the board, sir.
—Can you do them yourself? Stephen asked.
listened, scraped up the earth, listened, scraped and scraped.
lumberroom: the hollow knock of a ball and calls from the field.
darkness shining in brightness which brightness could not comprehend.
—Do you understand now? Can you work the second for yourself?
him and hid from sight of others his swaddling bands.
tyranny: tyrants, willing to be dethroned.
—It is very simple, Stephen said as he stood up.
—Yes, sir. Thanks, Sargent answered.
copybook back to his bench.
as he followed towards the door the boy's graceless form.
In the corridor his name was heard, called from the playfield.
—Run on, Stephen said. Mr Deasy is calling you.
turned his angry white moustache.
—What is it now? he cried continually without listening.
—Cochrane and Halliday are on the same side, sir, Stephen said.
—What is the matter? What is it now?
round him, the garish sunshine bleaching the honey of his illdyed head.
rare moustache Mr Deasy halted at the table.
—First, our little financial settlement, he said.
laid them carefully on the table.
—Two, he said, strapping and stowing his pocketbook away.
A sovereign fell, bright and new, on the soft pile of the tablecloth.
is for shillings. Sixpences, halfcrowns. And here crowns. See.
He shot from it two crowns and two shillings.
—Three twelve, he said. I think you'll find that's right.
haste and putting it all in a pocket of his trousers.
—No thanks at all, Mr Deasy said. You have earned it.
—Mine would be often empty, Stephen said.
Shakespeare say? Put but money in thy purse.
He lifted his gaze from the idle shells to the old man's stare.
but an Englishman too. Do you know what is the pride of the English?
history is to blame: on me and on my words, unhating.
—That on his empire, Stephen said, the sun never sets.
tapped his savingsbox against his thumbnail.
that? I owe nothing. Can you?
Mulligan, nine pounds, three pairs of socks, one pair brogues, ties.
Curran, ten guineas. McCann, one guinea. Fred Ryan, two shillings.
weeks' board. The lump I have is useless.
—For the moment, no, Stephen answered.
Mr Deasy laughed with rich delight, putting back his savingsbox.
it. We are a generous people but we must also be just.
—I fear those big words, Stephen said, which make us so unhappy.
Stephen sketched a brief gesture.
all Irish, all kings' sons.
 The rocky road to Dublin.
A gruff squire on horseback with shiny topboots. Soft day, sir John!
to Dublin. Lal the ral the ra. Lal the ral the raddy.
with some of your literary friends. I have a letter here for the press.
Sit down a moment. I have just to copy the end.
off some words from the sheet on the drum of his typewriter.
common sense. Just a moment.
sometimes blowing as he screwed up the drum to erase an error.
nuzzling thirstily her clove of orange.
Shouts rang shrill from the boys' playfield and a whirring whistle.
to be slightly crawsick? Jousts. Time shocked rebounds, shock by shock.
a shout of spearspikes baited with men's bloodied guts.
—Now then, Mr Deasy said, rising.
He came to the table, pinning together his sheets. Stephen stood up.
industries. Liverpool ring which jockeyed the Galway harbour scheme.
was no better than she should be. To come to the point at issue.
—I don't mince words, do I? Mr Deasy asked as Stephen read on.
Mürzsteg, lower Austria. Veterinary surgeons. Mr Henry Blackwood Price.
question. In every sense of the word take the bull by the horns.
Thanking you for the hospitality of your columns.
He raised his forefinger and beat the air oldly before his voice spoke.
destruction. Old England is dying.
broad sunbeam. He faced about and back again.
—Dying, he said again, if not dead by now.
 Shall weave old England's windingsheet.
or gentile, is he not?
years of wandering and, patient, knew the dishonours of their flesh.
—Who has not? Stephen said.
—What do you mean? Mr Deasy asked.
sideways open uncertainly. Is this old wisdom? He waits to hear from me.
From the playfield the boys raised a shout. A whirring whistle: goal.
What if that nightmare gave you a back kick?
history moves towards one great goal, the manifestation of God.
—A shout in the street, Stephen answered, shrugging his shoulders.
between his fingers. Looking up again he set them free.
end of my days. But I will fight for the right till the end.
 And Ulster will be right.
Stephen raised the sheets in his hand.
—A learner rather, Stephen said.
And here what will you learn more?
Mr Deasy shook his head.
Stephen rustled the sheets again.
—As regards these, he began.
see if you can get it into your two papers. What are they?
answer that letter from my cousin.
—Good morning, sir, Stephen said, putting the sheets in his pocket.
like to break a lance with you, old as I am.
—Good morning, sir, Stephen said again, bowing to his bent back.
hearing the cries of voices and crack of sticks from the playfield.
me a new name: the bullockbefriending bard.
Running after me. No more letters, I hope.
—Yes, sir, Stephen said, turning back at the gate.
Mr Deasy halted, breathing hard and swallowing his breath.
that? No. And do you know why?
He frowned sternly on the bright air.
—Why, sir? Stephen asked, beginning to smile.
—Because she never let them in, Mr Deasy said solemnly.
his lifted arms waving to the air.
stamped on gaitered feet over the gravel of the path. That's why.


On February 2, Omnivore Recordings will release the third and fourth discs in their splendid compilation series The Ru-Jac Records story. Ru-Jac was a Baltimore-based soul and R&B label founded by Rufus Mitchell and Jack Bennett (hence the label name) that began operations in 1963 and continued into the 1970s. The label featured better-known artists like Winfield Parker and Gene & Eddie (Omnivore has already released CDs devoted to the work of these artists) along with many lesser but should have been better-known artists.
Cheryl Pawelski, Altadena, California. 21 January 2015.
Cheryl Pawelski is a co-founder of Omnivore. Her music business career has been focused on preserving, curating and championing historic music and has included stints at Rhino Entertainment, Concord Music Group, and Capitol-EMI Records. Her many accomplishments include supervision and production of reissues and box sets by artists like Miles Davis, Aretha Franklin & King Curtis, Otis Redding, John Coltrane, the Staple Singers, and many more. Cheryl has also served as a Governor and Trustee of the Recording Academy and she is currently on the Board of Directors of the Blues Foundation.
Recently, I discussed The Ru-Jac Records Story releases with Cheryl who co-produced the Ru-Jac reissue series with Kevin Coombe.
Kevin Coombe has provided extensive liner notes for each of the four volumes. Together they lay out the history of Ru-Jac Records. What is the cliff notes version?
The Baltimore soul/R&B label Ru-Jac Records was founded in 1963 by local promoter Rufus Mitchell and investor partner Jack Bennett (their names forming the Ru-Jac label name). The label primarily released regional soul/R&B singles from 1963 until the mid-1970s, when Mitchell stepped away to focus on another business venture. A few tracks had been licensed throughout the years, but until now, there have been no comprehensive collections of the Ru-Jac label.
How did Omnivore come to acquire the rights to the Ru-Jac catalog?
A music attorney friend of mine had deep ties to the Ru-Jac catalog. While there had been offers in the past to purchase the catalog, he and the owners had rejected those. We'd worked together before and he thought we'd be a good home. Turns out, I think he was right! We're so grateful to be the caretaker of this music. It's a great responsibility and a great joy. There are so many terrific songs.
Omnivore previously released discs focused on Ru-Jac artists Winfield Parker and Gene & Eddie. What was the thinking in regard to releasing these discs before the multi-artist compilations?
They were the biggest artists on the label and the most recorded. We thought it'd be great to get those out first before diving into the overall story which naturally took longer. There were lots of tapes and acetates to transfer and try to identify, nothing being marked well, of course. So while we were sorting and figuring out as much as we could of the material emanating from the sources, we thought it'd be best to re-introduce Ru-Jac with Winfield Parker (a consulting producer on the whole reissue program) and Gene & Eddie with Sir Joe first.
While you were preparing these compilations was there one artist you were previously unfamiliar with who impressed you, or maybe one you hadn't heard for awhile who surprised you?
There were many. The Teardrops Band featuring Marie Allen just shreds. I love the Mask-Man and the Cap-Tans tracks. There are so many great tracks, some by completely unknown, unnamed artists. Notable to me are Celestine, Brenda Jones, The Jolly Jax, Rita Doryse, Kitty Lane, Leon Gibson, Dynamic Corvettes, so many – just jump in a let it rip, these are fun!
The liner notes include capsule biographies of the Ru-Jac artists. Is there one great Ru-Jac story, in the notes or not, that you love?
The thing that struck me the most (and to be certain, I don't love it), and it's still, sadly, so relevant today is the origin story. Rufus Mitchell, the owner of the label, was a promoter who was booking the segregated beach stages on the east coast. This label has the same sad story that Stax does, not as politically developed musically, and certainly lacking the bigger audience that hits afforded Stax, but the music came from the same place, the African American community. I find it intolerably sad and infuriating, the racial divides that existed then and persist and are being stoked now. It makes want to protect and preserve this music even more. Because of the cultural/political origins of Ru-Jac, I feel besides the super fun nature of the music, we also have a responsibility to tell the story of the artists and people involved and hand the stories and the music down, and not let it be lost to history.
Can we look forward to more Ru-Jac music from Omnivore?
This is pretty much it. It was a singles-only label, so we've restored what we could from what we have. If more tapes materialize, for sure, I'd love to do a volume five of odds and sods that might be found in the future, but right now, this is pretty much it. We are working on a collection of demos by Arthur Conley. He was the singer on the Ru-Jac Harold Holt single, but I found all these demos in the Ru-Jac tapes and despite their audio compromises, the songs are simply beautiful. Some are just solo piano demos with him singing, some have a little combo. Later he cut some of the songs he was writing during this time for Jotis, Fame, and Atco, but there are a bunch of previously unknown compositions. If the songs weren't so cool, we wouldn't bother because the audio quality may not be brought up to our usual standards. We're working on it now, but frankly, I can't get some of the tunes out of my head. That tells me a whole lot. These are intimate and magical little performances in a very workmanlike setting. In one, a phone rings in the middle of the song, a few he announces who he is and the song title at the beginning. It's fly on the wall stuff and while listening your imagination gets enough clues to paint the scene. I hope folks like them as much as I do.
Provide a brief history of Omnivore. Where did you come from? How long has the label been around? What is your mission as a company? In terms of soul and R&B, what have you done so far and what can fans look forward to?
Omnivore is a label, publisher, licensing and consulting group of industry veterans that came together eight years ago to form a company primarily focused on the preservation and release of older recordings. Focusing as much as possible on great or important recordings that were never previously issued or those left behind or overlooked as the business and configurations rapidly changed over the course of the last 50 years. We're not interested in genres, we interested in great music. As far as soul/R&B, in the past, we've released albums by Arthur Alexander, The Blind Boys Of Alabama, The Bo-Keys, Darondo, Carl Hall, MC Lyte, Bobby Patterson and Bobby Rush. We also just produced a Nina Simone release for BMG that will be released in early February. Looking forward, you never know, we'll be as surprised as the fans are – that's all part of the fun.


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text:
CinemaTalk: a Conversation with Michael Berry
dGenerate Films presents CinemaTalk, an ongoing series of conversations with esteemed scholars of Chinese cinema studies. These conversations are presented on this site in audio podcast and/or text format. They are intended to help the Chinese cinema studies community keep abreast of the latest work being done in the field, as well as to learn what recent Chinese films are catching the attention of others. This series reflects our mission to bring valuable resources and foster community around the field of Chinese film studies.
In this conversation with dGenerate's Kevin Lee, Michael shares his insights on Jia Zhangke, specifically his career development since the "Hometown Trilogy" and his recent controversy at the Melbourne International Film Festival. Be sure to read Jia's statement of withdrawal from the Melbourne Film Festival as a point of reference.
Play the Podcast (Time: 17:39)
Download it here (right-click to download, file size: 8.2 MB).
Get a list of Michael's publications and a timecoded index of topics covered in the interview after the jump.
Interview Topic Index
0:00-0:51 – Introduction 0:51-4:00 – Jia Zhangke's career development 4:00-7:45 – Jia's recent controversy at Melbourne 7:46-11:45 – Jia as a political filmmaker 11:45-15:20 – Moving beyond the mavericks 15:20-17:30 – Distributing the digital revolution
Selected Publications by Michael Berry
Jia Zhang-ke's Hometown Trilogy (British Film Institute & Palgrave Macmillan, forthcoming 2009)
A History of Pain: Trauma in Modern Chinese Literature and Film (Columbia University Press, 2008)
Speaking in Images: Interviews with Contemporary Chinese Filmmakers (Columbia University Press, 2005; Traditional Chinese edition, Rye Field, 2007; Simplified Chinese Edition, Guangxi Normal University Press, 2008)
Book Length Translations by Michael Berry
The Song of Everlasting Sorrow: A Novel of Shanghai, by Wang Anyi. Translation by Michael Berry and Susan Chan Egan, with an Afterword by Michael Berry (Columbia University Press, 2008).
To Live by Yu Hua. Translation and Afterword by Michael Berry (Anchor Books, 2003).
Nanjing 1937: A Love Story by Ye Zhaoyan. Translation and introduction by Michael Berry (Columbia University Press, 2002, Faber & Faber, 2003, Anchor Books, 2004).
Wild Kids: Two Novels about Growing Up by Chang Ta-chun. Translation and introduction by Michael Berry (Columbia University Press, 2000).
#chinesecinema #michaelberry #interview #educationalresource #podcast #jiazhangke #melbourneinternationalfilmfestival #filmstudies #academic #jiazhangke #cinemastudies
A NEW OLD PLAY featured in Cinema Scope Magazine


Every so often there is another round of a fairly unsophisticated SQL injection that places malware scripts into poorly coded websites occurs and then there is a enviably a security company that hypes the infections and flood of new stories about it. Another round of the infection occurred in the last week, dubbed Lizamoon by Websense who is the company to hype this round (we previously discussed Websense's false claims of WordPress security issues). From what we have seen dealing with malware infected websites and other data confirms is that these "massive" infections are not massive as they are claimed to be each time, in fact they are of average size for a malware infection of websites. Most of those average size malware infections never receive any press coverage. The reason these attacks seems to receive the coverage is because of the use of Google search results to provide a large but highly inaccurate measure of the size of the infection.
The most important thing to understand about these infections, and this often not mentioned, is that they are completely preventable by properly sanitizing user input data that will be sent to a database. Anyone coding should be well aware of this the possibility of a SQL injection , these specific attacks have been occurring for years, and take the necessary precautions. Prevent SQL injections is one of key things mentioned in our article on securing your website from hackers. Widely used software like WordPress, Drupal, and Joomla are not susceptible to such a basic SQL injection. Unfortunately, even websites that get hit often don't bother to take the necessary precautions to prevent these SQL injections. Instead, they often just remove the code from the database. There are also unethical website malware removal companies that will remove the infection from the database without insuring the SQL injection vulnerability has been fixed.
.Because the code has been escaped it will appear as text in the pages and therefore be searchable. When the code is placed into the website in escaped form it is not infectious.
The number that Google provides in an estimate, it's not all clear how accurate it is. If you include duplicate pages currently you can only see 604 results for the search "<script src=http://lizamoon.com/ur.php></script>" despite there being "about 1,470,000 results".
The number includes any page, like this one, that mentions the code.
Not all pages that have the code are actually infection, because the code only searchable if it escaped. So it would require that another instance that is not escaped be one the page for it to be infectious. We checked the first 10 results for the search "<script src=http://lizamoon.com/ur.php></script>" which were still injected and found that only four of them were infectious.
Most malware infections are not measurable using search results making a comparison with them impossible using the metric.
Web pages are not a good measure of the reach of a malware infection. A page could be accessed millions of times a day or never.
The ideal way to measure the size of a malware infection would be to determine how many times each pages with the malware would be accessed. There is not a tool able to do this and there is unlikely to be one. What we have found to best indicator available to measure the size of a malware infection size is Google Safe Browsing system. This system scans web pages from across the Internet for malware. This data is used to block infected websites in Google's search results and is also used for malware protection in the FireFox, Chrome, and Safari web browsers. It does not scan all websites and does not scan all of the websites it does scan equally, so the number won't include every infected website. Google doesn't indicate what criteria it uses to determine how often it scan various, but in general it scans more popular website more often so it should provide a good measure of how many website that people are likely to access were infected. At the moment the system reports that lizamoon.com has infected 1436 domains. That is far lower than the nearly 4 million websites claimed to have been infected according to one source, far lower than the 1,470,000 reported for a search on "<script src=http://lizamoon.com/ur.php></script>", and far lower than "hundreds of thousands of domains" claimed by Websense. By comparison, the IP address 86.55.140.203 that is called by a infection that has recently been hitting many osCommerce based websites is reported to have acted as an intermediary for 2957 sites.


text:
\section*{{Program Summary}}
{\em Title of the Programs:} phi3\\

\noindent
{\em Computer:} Sun 19\\

\noindent
{\em Operating system:} Unix\\

\noindent
{\em Programming language used:} FORTRAN 77\\

\noindent
{\em Peripherals used:} Laser Printer\\

\noindent
{\em Number of lines in distributed program:} 1510\\

\noindent
{\em Keywords:}  Nonperturbative, bound states, Feynman-Schwinger
representation, Monte-Carlo, numerical evaluation.\\

\noindent
{\em Nature of physical problem:}\\
The program provided here evaluates the mass and distribution probabilities
of the fully interacting n-body propagator ($n\le 3$) for scalar $\chi^2\phi$
interaction in 3+1 dimensions. The evaluation takes into account {\em all self
energy, vertex dressing, and exchange interaction} contributions except those involving matter loops (the quenched approximation).
\\

\noindent
{\em Method of solution:}\\
The Feynman-Schwinger representation approach is used to express the
field theoretical Green's function in terms of a quantum mechanical path
integral. The resultant expression is evaluated using a Monte-Carlo simulation.
\\

\noindent
{\em Restrictions of the program:}\\
Only $n=1,2$, and $3$ body propagators are considered. The extension to
$n\ge 4$ requires straightforward modifications in the program.
\\

\noindent
{\em Typical running time:}\\
About 1 day for the 1-body propagator with the self energy.

\section*{{\bf LONG WRITE-UP}}

\section{Introduction}

In nuclear physics one is often faced by problems that require nonperturbative
 methods. The best known example is the problem of bound states. Even if the
underlying theory may have a small coupling constant (such as in QED), and
therefore allows the use of perturbation theory in general, the treatment of
bound states are inherently nonperturbative. The n-body bound state is defined
by the pole of the interacting n-body propagator. A perturbative approximation
of n-body propagator does not produce the bound state pole location.
Therefore it is essential that reliable nonperturbative methods that take all
orders of interaction into account are developed. For this reason, numerous
nonperturbative methods have been developed and successfully used in the
literature. Some of the best known examples are lattice gauge
theory~\cite{ROTHE} (LGT), and relativistic bound state
equations~\cite{NAKANISHI,TJON0,GROSS1}.

In a recent paper~\cite{SAVKLI1} we (along with authors J. Tjon, and F.
Gross) have discussed yet another method known as the Feynman-Schwinger
representation(FSR). The basic idea in the FSR
approach~\cite{SAVKLI1,SIMONOV1,TJON1,BRAMBILLA} is to integrate out all
fields at the expense of introducing quantum mechanical path integrals over
the {\em trajectories of particles}. Replacing
the path integrals over fields with path integrals over trajectories has an
enormous computational advantage. The advantage is due to the fact that
the path integration over trajectories involves a variation of {\em lines}
rather than {\em fields in a volume}. Therefore the degrees of freedom is
considerably fewer. The FSR approach differs from the LGT in that it utilizes
a space-time continuum, therefore maintaining the Poincare symmetry.
On the other hand it should be pointed out that the FSR approach is not
without its drawbacks. In particular, how to extend the FSR approach to
include fermions is not known. In the past
researchers~\cite{BRAMBILLA,SIMONOV2,SIMONOV3} have attacked the fermion
problem using various approximations. An {\em exact } result involving
fermions is an important problem and requires further study.

While being able to calculate a nonperturbative result by itself is
interesting, an additional motivation in studying the FSR approach is to
determine which subsets of diagrams give the dominant contribution to the
n-body propagator. This is particularly important in determining what kind of
approximations are reasonable within the context of bound state equations. An
example of how the FSR results can be used to compare different
nonperturbative approximation schemes was presented in
Refs~\cite{SAVKLI1,SAVKLI2}. In those works the emphasis was on the
development of the formalism and application to the 1 and 2-body propagators.
In Ref~\cite{SAVKLI2}, The FSR prediction for the
1-body mass in Scalar QED was compared by the rainbow-Dyson-Schwinger
equation prediction. It was found~\cite{SAVKLI2} that while the FSR approach
provides a real mass pole for all coupling strengths, the Dyson-Schwinger
equation provides a complex mass pole beyond a critical coupling strength.
Furthermore it was found that, for Scalar QED in 0+1 dimension,  the vertex
corrections to the exchange interaction do not contribute to the 2-body
binding energy~\cite{SAVKLI2}. These examples demonstrate the potential
usefulness of the FSR approach. The knowledge about the nonperturbative
propagators and vertices provided by the FSR is valuable as an input in
testing and improving the modeling of other nonperturbative approaches such
as Dyson-Schwinger equations.~\cite{ROBERTS1,SAVKLI0}

The two and three-body bound state sectors provide possibilities for the
application of the FSR formalism. In particular it is
important to see how various bound state equations (such as Bethe-Salpeter, Gross (spectator), Blankenbekler-Sugar, Equal-time, and nonrelativistic)
compare with the quenched FSR results. Applications of the FSR approach to 2
and 3 body states with comparisons to various bound state equation results in
$\chi^2\phi$ theory is currently under study and will be
presented in a separate article.~\cite{SAVKLI3}

In this paper we present a complete numerical algorithm for the evaluation
of $n$-body masses ($ n\le 3 $) and distribution probabilities for scalar
$\chi^2\phi$ interaction in 3+1 dimensions. By providing this algorithm
we intend to facilitate the comparison of various nonperturbative
methods with the exact quenched results in $\chi^2\phi$ theory.
The organization of the paper is as follows: In the next section we present a
brief summary of the FSR formalism. In the third section, using various
1, 2, and 3-body cases as examples, we discuss how results are obtained. And
in the fourth section we explain the components of the program.

\section{The Feynman-Schwinger representation for scalar fields}

We consider the theory of charged scalar particles $\chi$ of mass $m$
interacting through the exchange of a neutral scalar particle $\phi$ of mass
$\mu$. The Euclidean Lagrangian for this theory is given by
\begin{equation}
{\cal L}_E=\chi^*\bigl[m^2-\partial^2+g\phi\bigr]\chi+\frac{1}{2}\,\phi(\mu^2-\partial^2)\phi.
\label{lagr0}
\end{equation}
The two body Green's function for the transition from the initial state
$\Phi_{i}=\chi^*(x)\chi(\bar{x})$ to final state $\Phi_{f}=\chi^*(y)\chi(\bar{y})$ is given by
\begin{equation}
G(y,\bar{y}|x,\bar{x})=N\int {\cal D}\chi^*\int {\cal D}\chi\int {\cal D}\phi
\,\Phi^*_f\Phi_i\,e^{-S_E}.
\label{g0}
\end{equation}
The final result for the two-body propagator
involves a quantum mechanical path integral that sums up contributions coming
from all possible {\em trajectories} of {\em particles}
\begin{equation}
G=-\int_0^\infty ds \int_0^\infty d\bar{s} \int ({\cal D}z)_{xy}\int ({\cal D}\bar{z})_{\bar{x}\bar{y}}\,e^{-S[Z]},
\label{g1.phi3}
\end{equation}
where $S[Z]$ is given by
\begin{equation}
S[Z]\equiv -iK[z,s]-iK[\bar{z},\bar{s}]+V_{0}[z,s]+2V_{12}[z,\bar{z},s,\bar{s}]+V_{0}[\bar{z},\bar{s}].
\label{action}
\end{equation}
where
\begin{eqnarray}
K[z,s]&=&(m^2+i\epsilon)s-\frac{1}{4s}\int_0^1 d\tau \,\frac{dz_\mu(\tau)}{d\tau}\frac{dz^\mu(\tau)}{d\tau},\label{k1}\\
V_{0}[z,s]&=&\frac{g^2}{2}s^2\int_0^1d\tau\int_0^1d\tau' \,\Delta(z(\tau)-z(\tau'),\mu),
\label{v0.phi3}\\
V_{12}[z,\bar{z},s,\bar{s}]&=&\frac{g^2}{2}s\bar{s}\int_0^1d\tau\int_0^1d\bar{\tau}\, \Delta(z(\tau)-\bar{z}(\bar{\tau}),\mu).\label{v12.phi3}
\end{eqnarray}
Here the $V_{0}[z,s]$ term represents the self energy contribution, while
the $V_{12}[z,\bar{z},s,\bar{s}]$ term represents the exchange interaction (Fig.~\ref{trajectory}).
The interaction kernel $\Delta(x)$ is defined by
\begin{eqnarray}
\Delta(x,\mu)&=& \int \frac{d^4p}{(2\pi)^4}\frac{e^{ip\cdot x}}{p^2+\mu^2}=\frac{\mu}{4\pi^2|x|}K_1(\mu|x|).
\label{kernel.phi3}
\end{eqnarray}
While we present expressions for the 2-body case, generalization
to an arbitrary n-body system is trivial.
The bound state spectrum can be determined from the spectral decomposition of the two body Green's function
\begin{equation}
G(T)=\sum_{n=0}^{\infty}c_ne^{-m_nT},
\end{equation}
where T is defined as the average time between the initial and final states
\begin{equation}
T\equiv\frac{1}{2}(y_4+\bar{y}_4-x_4-\bar{x}_4).
\label{tdef}
\end{equation}
In the limit of large $T$, the ground state mass is given by
\begin{equation}
m_0=\lim_{T\rightarrow\infty}-\frac{d}{dT} ln[G(T)]=\frac{\int {\cal D}Z S'[Z]e^{-S[Z]}}{\int {\cal D}Z e^{-S[Z]}},
\label{groundstate}
\end{equation}
While this result in principle is correct, the convergence to the asymptotic
mass is slow due to the continuum contribution. The spectrum of the particle
involves the mass pole and a cut beyond this pole representing the continuum
contribution. Assuming that the constituents of the bound state are restricted
to be at equal times in the initial and final states, the Green's function
can be written as a function of time $T$, total displacement ${\bf R}$, and
relative coordinate ${\bf r}$, G(T,{\bf R},{\bf r}).\footnote{Dependence
on the initial relative final coordinate ${\bf r}_0$ is implicit.}

In order to eliminate the contribution of continuum states, introduce the
Fourier transform,
\begin{equation}
\tilde{G}(T,{\bf P},{\bf p})=\int d^3{\bf R}\, d^3{\bf r}\, e^{i{\bf P}\cdot{\bf R}+i{\bf p}\cdot{\bf r}}G(T,{\bf R},{\bf r})
\end{equation}
where ${\bf P}$ is the CM momentum, and ${\bf p}$ is the relative momentum between particles. Setting both ${\bf P}={\bf p}=0$ one has
\begin{equation}
\tilde{G}(T,0,0)=\int d^3{\bf R}\, d^3{\bf r} \, G(T,{\bf R},{\bf r}),
\end{equation}
which eliminates the contribution of the continuum and projects out the s-wave
state. While an integration over ${\bf r}$ is not necessary for the elimination
of the continuum contribution, it is useful in eliminating the
contribution of states with nonzero orbital angular momentum.

While the result for the Green's function Eq.~\ref{g1.phi3} is exact in the
quenched approximation, due to its oscillatory behavior it is not
appropriate for Monte-Carlo simulation. In Ref.~\cite{SAVKLI1} it was shown
that one can perform a Wick rotation in variable $s$ to avoid these
oscillations. In the limit $g^2\rightarrow 0$ the dominant
contribution to the integral in Eq.~(\ref{g1.phi3}) can be shown, by using the
saddle point method, to come from
\begin{equation}
s=is_0=i\frac{T}{2m}.
\end{equation}
Since the large $s$ values do not contribute to the integral even without
 the interaction term, it is a good approximation to suppress the $g^2$ term
at large s values. While this suppression is done it is important that
the integrand is not modified in the region of dominant contribution
$s\sim is_0$. This can be achieved by scaling the $s$ variable, {\em in the interaction term only}, by
\begin{equation}
s\rightarrow \frac{s}{R(s,s_0)},
\label{sredef}
\end{equation}
where
\begin{equation}
R(s,s_0)\equiv 1-(s-is_0)^2/\Gamma^2.
\label{rdef}
\end{equation}
In the free case, $(g^2=0)$, the width $W$ of the region of dominant $s$
contribution goes as
\begin{equation}
W=\sqrt{\frac{T}{2m^{3}}}.
\label{width}
\end{equation}
Therefore, in the free case the dominant contribution to the $s$ integral
comes from $i(s_0-W)<s<i(s_0+W)$. This claim is supported by the Monte-Carlo
simulation results. In Fig.~\ref{sdist} we present the results for
$s$-distributions for two different coupling strengths for time $T=40$, and
$m=1$ GeV. According to the estimate given above Eq.~(\ref{width}), for $g=0$,
the dominant contribution to the  $s$-distribution comes from the region
$15.53<s<24.47$ which is in agreement with the result presented in
Fig.~\ref{sdist}.
In order to ensure that the scaling given in Eq.~(\ref{sredef}) does not make
a significant change in the region of dominant contribution, $\Gamma$ should
be chosen such that
\begin{equation}
\Gamma\ge W
\end{equation}
As one increases the coupling strength, the value of $s_0$ deviates
from its free value. Therefore, in general, $s_0$ has to
be defined self consistently by monitoring the peak of the $s$ distribution.
In Figure~\ref{sdist} we display the s-distribution for two different coupling
strengths. It is seen that as the coupling strength is increased the peak of
the s-distribution moves towards higher s values. In general the peak of the
distribution can be parameterized as
\begin{equation}
s_0=C\frac{T}{2m}.
\label{stationary}
\end{equation}
The dependence of $C$ on coupling strength $g^2$ is determined self
consistently. In Fig.~\ref{speak} $C$, which gives the location of the stationary point through Eq.~(\ref{stationary}), is plotted as a function of the
coupling strength $g^2$. According to Fig.~\ref{speak}, it is not possible to
find a self consistent stationary point beyond the critical
coupling strength of $g^2=31$ GeV$^2$. A similar critical behavior was also
observed in Refs.~\cite{ROSY} within the context of a variational approach.

The insensitivity of the dressed mass to the width $\Gamma$ has been
investigated~\cite{SAVKLI1} and found that a choice of $\Gamma^2=2W^2$ was
satisfactorily large. Results presented here employ the same value of $\Gamma$.

Prescription given by Eqs.~(\ref{sredef}), and (\ref{rdef}) enables one to
perform a Wick rotation in variable $s$ to obtain a finite and non-oscillatory
expression for the fully interacting two-body propagator:

\begin{eqnarray}
G&=&\int_0^{\infty} ds \int_0^{\infty} d\bar{s} \int ({\cal D}z)_{xy}\int ({\cal D}\bar{z})_{\bar{x}\bar{y}}\label{g2}\\
&&\times{\rm exp}\biggl[-K[z,s]-K[\bar{z},\bar{s}]+V_0[z,s_r]+V_0[\bar{z},\bar{s}_r]+2V_{12}[z,\bar{z},s_r,\bar{s}_r]\biggr],\nonumber
\end{eqnarray}
where
\begin{equation}
s_r\equiv \frac{s}{R(s,s_0)}.
\end{equation}
The path integral is discretized using
\begin{equation}
({\cal D})_{xy}\rightarrow(N/4\pi s)^{2N}\Pi^{N-1}_{i=1}\int d^4z_i,
\end{equation}
where the s-dependence is critical in obtaining the correct normalization.
Note that the integration over the final coordinates is not included in this
expression.

The discretized versions of kinetic and interaction terms are given by
\begin{eqnarray}
K[z,s]&\rightarrow& (m^2+i\epsilon)s-\frac{N}{4s}\sum_{i=1}^{N}(z_i-z_{i-1})^2,\\
V_0[z,s]&\rightarrow&\frac{g^2s^2}{2N^2}\sum_{i,j=1}^{N}\Delta(\frac{1}{2}(z_i+z_{i-1}-z_j-z_{j-1}),\mu),\\
V_{12}[z,\bar{z},s,\bar{s}]&\rightarrow&\frac{g^2s\bar{s}}{2N^2}\sum_{i,j=1}^{N}\Delta(\frac{1}{2}(z_i+z_{i-1}-\bar{z}_j-\bar{z}_{j-1}),\mu).
\end{eqnarray}

We next address the regularization of the ultraviolet (short distance)
singularities. The ultraviolet singularity in the kernel $\Delta(x,\mu)$
Eq.~(\ref{kernel.phi3})
can be regularized using a Pauli-Villars regularization prescription. In order
to do this one replaces the kernel
\begin{equation}
\Delta(x,\mu)\longrightarrow \Delta(x,\mu)-\Delta(x,\alpha\mu),
\end{equation}
where $\alpha$ is in principle a large constant. The ultraviolet
singularity in the interaction is of the type
\begin{equation}
\int dz\, z\, \Delta(z,\mu).
\end{equation}
At short distances the kernel $\Delta(z,\mu)$ goes as $1/z^2$. Therefore,
the self energy calculation involves a logarithmic type singularity. The
Pauli-Villars regularization takes care of this singularity. The
Pauli-Villars regularization is particularly convenient for Monte-Carlo
simulations since it only involves a modification of the kernel. In order to
achieve an efficient convergence in numerical simulations we use a rather
small cut-off parameter $\alpha=3$. This choice leads to a less singular
kernel. The value of $\alpha$ can be increased arbitrarily at the cost
additional computational time. It should be noted that while we employ a
Pauli-Villars regularization throughout this paper, in general,
the bound state problem {\em without} self energies {\em does not} have any
UV singularities. UV singularities are only associated with the self energies
of the particles. After this brief summary of the formalism, in the next
section we present some of the results and discuss the details of the
algorithm.

\section{Running the code: applications}

The Monte-Carlo simulation starts by choosing an initial configuration
for the trajectories of the particles. The choice of the initial
trajectory is arbitrary (except at the end points). In Fig.~\ref{termalize}
the evolution of the action as a function of number of updates
for two different initial conditions is displayed. Starting with a random
initial trajectory is analogous to a high temperature system and the
termalization
(reaching to the ground state) takes a long time (about 1000 updates). However
if one starts by a classical free trajectory, the initial configuration is
analogous to a frozen system without any fluctuations and the termalization
results in an increase of the action. However asymptotically both results
should converge as shown in Fig.~\ref{termalize}. We usually start with an
orderly system and disregard the first 1000 updates. Step sizes of the random
walker in configuration space and in s-space should be chosen such that
the average acceptance rate of Monte-Carlo updates are about \% 50. In each
run we typically make 500000 updates of trajectories. In order to reduce the
statistical errors runs must be repeated (usually more then 10 times) using
different random number seeds. The correlation function $X(n)$ of sampled
configurations in each run is defined as
\begin{equation}
X(n)\equiv\frac{\left< m(i) m(i+n) \right> - \left< m \right>^2 }{\left< m
\right>^2 },
\end{equation}
where $m(i)$ is the mass measurement at the $i$'th update. The correlation
function $X(n)$ measures how the information about a given configuration is
lost as a function of the number of updates $n$. In Figure~\ref{correlation}
we show the correlation function for the 1-body problem. According to
Fig.~\ref{correlation} the number of updates necessary for the correlation
between sampled trajectories to vanish is around $n=1000$. The number of
configurations sampled in our simulations, which is around 500000, is well
above the correlation length 1000, thereby insuring that uncorrelated
trajectories are sampled during the Monte-Carlo integration.

The time $T$ required to reach to the asymptotic limit
increases as  $g^2$ increases. For $g^2=25$ the asymptotic value of the mass,
given by Eq.~(\ref{groundstate}),
is obtained around $mT=40$. In particular for the result shown in
Fig.~\ref{mvsg2.1b}, as $g^2$ ranged from $g^2=0$ GeV$^2$ to $g^2=31$ GeV$^2$
the asymptotic time values used were increased from $mT=35$ to $mT=45$. As
time $T$ is increased the number of steps $N$ should also be proportionally
increased so that the step size of the particle trajectory remains the same.
As one increases the coupling strength $g^2$, trajectories of the particles
deviate from the classical trajectory to a greater degree. This increase in
fluctuations requires that one uses a higher $N$ value. The number of steps
$N$ particles take between the initial and final coordinates is typically
chosen to be $35<N<45$.

In Fig.~\ref{mvsg2.1b} the $g^2$ dependence of the one-body dressed
mass is presented. 1-body masses presented here are lower than those in \cite{SAVKLI1}. This is due to the fact that in that work $C$ was assumed
to be approximately 1. However it was subsequently realized that $C$ deviates
from 1 significantly (see Fig.~\ref{speak}) as coupling strength is increased,
and a self consistent determination of $C$ is important to pin down the
critical point.  According to Fig.~\ref{speak} there is no self consistent
stationary point Eq.~(\ref{stationary}) beyond the critical coupling strength
$g^2=31$ GeV$^2$, and the 1-body dressed mass becomes unstable for
$g^2>31$ GeV$^2$ (Fig.~\ref{mvsg2.1b}).

Next two applications involve the two and three-body bound
states of equal mass particles. While the algorithm provided is capable to
take into account all self energy and vertex dressing corrections to the bound
state, in the bound state applications provided here the self energy
contributions of particles were not taken into account. This is controlled by
a switch in the input file (see Table~\ref{PARAMET} for input options). In
Fig.~\ref{mvsg2.2b} the $g^2$ dependence of the two-body bound state mass is
presented. Beyond the critical coupling strength of $g^2=100$ GeV$^2$ the
2-body mass becomes unstable. During the Monte-Carlo simulation the radial
distributions of particles are stored in histograms. In general for an n-body
bound state there are $n(n-1)/2$ relative distances. Since the particles are
assumed to have equal time coordinates in the final state, essentially the
relative distance is equal to the spatial distance. Let $r_{ij}=|r_i-r_j|$ be
the distance between particles $i$ and $j$. In this case the histogram
$P_{ij}(r_{ij})$ stores the number of final state configurations sampled in
the interval $(r_{ij}-\delta/2,r_{ij}+\delta/2)$, where $\delta$ is the bin
size. The range of $r_{ij}$ values is specified in the program using
\begin{equation}
0< r_{ij} < \frac{20}{m_i+m_j}\ \ {\rm Fermi}.
\end{equation}
The choice of range is arbitrary as long as a reasonably smooth histogram is
produced. The number of bins in each histogram is chosen to be 100. Therefore
for two
particles of mass 1 GeV, the maximum radius to be histogrammed is 10 Fermi;
and the size of each bin is given by $\delta=0.1$ Fermi.
In Fig.~\ref{rdist.surf.2b} we present the projection of the radial
probability distribution onto a two-dimensional surface. The two-body
probability distribution, presented in Fig.~\ref{rdist.surf.2b}, shows
the result for $g^2=25$ GeV$^2$. Notice that the probability distribution
vanishes at the origin. This is due to the phase space factor $4\pi r^2$. In
order to be able to compare the probability distribution with a wave function
the phase space factor should be factored out. In general the radial wave
function {\em amplitude} $\Psi(r)$ is given by:
\begin{equation}
|\Psi(r)|=\sqrt{\frac{P(r)}{4\pi r^2}}
\label{phase}
\end{equation}
The normalization of the probability distribution histogram presented
in Fig.~\ref{rdist.2b} is arbitrarily fixed such that the maximum entry is
equal to 1.

In generating the surface plot (Fig.~\ref{rdist.surf.2b}), it is assumed
that one of the particles is fixed at the origin. The amplitude
of the surface gives the probability of finding the second particle at a
distance $r$.
While the surface plot for a two-body bound state is not necessary for
a visual understanding of the bound state structure, the three-body bound
state demands a three dimensional plot. In the three-body case there are
three relative coordinates. In order to be able to plot the three-body
probability distribution we fix the location of two of the particles
along the y axis, and calculate the probability of finding the third particle
in an arbitrary distance from two fixed particles. In Fig.~\ref{rdist.surf.3b}
we represent the probability distribution of the third particle for a given
fixed configuration of the first and second particles. Assume that the fixed
particles are particle 1 and particle 2. The probability distribution of
the third particle is given by
\begin{equation}
P_3(|{\bf r_3}|)\equiv P_{13}(|{\bf r_3-r_1}|)P_{23}(|{\bf r_3-r_2}|)
\end{equation}
Probability distribution $P_3(|{\bf r_3}|)$ includes the phase space contribution. Therefore $P_3(|{\bf r_3}|)$  represents
the probability of finding the third particle in a ring shown in
Fig.~\ref{ring.3b}. For example in the first plot of Fig.~\ref{rdist.surf.3b}
two fixed particles are very close to each other such that the third particle
sees them as a point particle. Therefore the probability distribution of
the first plot of Fig.~\ref{rdist.surf.3b} is very similar to the two-body
distribution given in  Fig.~\ref{rdist.surf.2b}. However as the fixed
particles are separated from each other the third particle starts having
a nonzero probability of being in between the two fixed particles (second
and third plots of Fig.~\ref{rdist.surf.3b}). Eventually when the
two fixed particles are kept away from each other the third particle has
a nonzero probability distribution only at the origin (the last plot
shown in Fig.~\ref{rdist.surf.3b}). In Fig.~\ref{rdist.3b} the {\em two-body}
distribution function $P_{12}$ in a three-body system is shown.  All of these
plots were produced with three equal particles of mass $1$ GeV, and the
coupling strength of $g^2=64$ GeV$^2$.

\section{Program details}
In this section we discuss the details of the program. We start by providing
the tables of input parameters~\ref{PARAMET} and arrays~\ref{ARRAY} and then
summarize the components of the program.

\subsection{Description of Input parameters}
\label{PARAMET}
\begin{flushleft}
\mbox{
\begin{tabular}{|l|l|} \hline
SIG = 1 GeV & Arbitrary momentum scale\\
\hline
IPAR(I)& I=1,2,3, Particles present  (0=n, 1=y)  \\
\hline
IEXCH(I,I)& I=1,2,3, Self  Interactions (0=n, 1=y)\\
\hline
IEXCH(I,J)& $(I,J)={(1,2),(1,3),(2,3)}$ Exch. Int. (0=n, 1=y) \\
\hline
QM(I) & Mass of particle I\\
\hline
G & The coupling strength\\
\hline
XMU & The exchange mass $\mu$\\
\hline
ALPHA & The Pauli-Villars mass ratio: $m_{pv}=\alpha$ $\mu$ \\
\hline
BETA = 1 & The width of $R(s,s_0)\equiv 1-\beta
(s-iC \hat{s}_0)^2/T^\gamma$ \\
\hline
GAMMA = 1 & The T dependence of the width.\\
\hline
C & The peak location of the s distribution s=$C \hat{s}_0$.\\
  &  C is determined self-consistently. \\
\hline
N & Number of steps along the trajectory \\
\hline
NSMPL & $\#$ of sampled trajectories in MC integration \\
\hline
NVOID & No. of uncounted samples for initial termalization \\
\hline
ZSTEP & Max. step size of the random walker in coord. space \\
\hline
SSTEP & Max. step size of the random walker in $s$ space \\
\hline
EPSA  & The short distance(UV) cut-off for preventing\\
                        &   explicit occurrence of 1/0.0 type of singularity.\\
                        &  This is not a regulator however. The UV \\
                        &  regularization is done using Pauli-Villars subtraction\\
\hline
IDUM & The seed of the random number generator \\
\hline
Z(I,0,J) & Initial coordinates of particle I=1,2,3   \\
\hline
Z(I,N,J) & Final coordinates of particle I=1,2,3  \\
\hline
IWRTA,IWRTM & Action, mass to be stored in file ? (0=n, 1=y)\\
\hline
INTOUT & Integrate over final coordinates ?\\
\hline
\end{tabular}
}
\end{flushleft}

\subsection{Arrays }\label{ARRAY}

\begin{flushleft}
\mbox{
\begin{tabular}{|l|l|} \hline
QM(3)  & Particle masses\\
\hline
IPAR(3)& Determines which particles are present. \\
\hline
   Z(3,0:400,4)& The trajectories of particles\\
\hline
ZNEW(3,0:400,4)& The updated trajectories of particles\\
\hline
SMAX(3) & The maximum value of s value to be histogrammed. \\
        &   (not an integration cut-off)\\
\hline
RMAX(3,3)& The maximum relative distance between particles\\
         & to be histogrammed. (not an integration cut-off) \\
\hline
SHIST(3,200)& Histogram of $s$ values \\
\hline
RHIST(3,3,200)& Histogram of relative distances between particles \\
\hline
SUMK(3) & Kinetic energies of particles\\
\hline
SUMV(3,3) & Potential energies of particles: SUMV(I,I): self\\
          & energy of the I'th particle, SUMV(I,J): the exchange \\
          & energy between I'th and J'th particles. \\
\hline
SUMKN(3)  & Updated kinetic energies\\
\hline
SUMVN(3,3) & Updated potential energies\\
\hline
\end{tabular}
}
\end{flushleft}

\subsection{Main Program}
The main program starts by calling the INPUT subroutine. This subroutine reads
input parameters described in Table~\ref{PARAMET}.
Next, subroutine XINTGR is called to perform the Monte-Carlo simulation. In
the following the role of each subroutine and function is explained.

\subsection{Subroutine INPUT}
In this subroutine 12 input parameters are read. In addition to
reading these parameters, histograms for the
radial and s distributions, and initial trajectories of the particles are
initialized. Initialization of trajectories is done using the classical
free trajectories of particles.

\subsection{Subroutine XINTGR }

 This subroutine {\em controls} basic steps of the Monte-Carlo sampling
process. First, the kinetic and the potential sums corresponding to the
initial trajectories of particles are calculated by calling the XSUMS
subroutine. Next step is the termalization process. In order to reach
termalization the configuration of trajectories are updated NVOID times by
calling the UPDATE subroutine. First NVOID updates are not used in the
actual calculation of the bound state mass or the probability distribution.
After the termalization the sampling is done for NSMPL times. The results
for the $s$ values and the relative distances of particles are
histogrammed. Finally the bound state mass is calculated.

\subsection{Subroutine UPDATE }

This subroutine is responsible for updating the current configuration
of trajectories. Each coordinate and $s$ parameter is updated once.
Samplings are done according to distribution
\begin{equation}
e^{-S[z]}
\end{equation}
distribution. If the ratio $r$,
\begin{equation}
r=e^{-(S[z']-S[z])},
\end{equation}
is larger than 1 updates are always accepted. When $r<1$ the update is
accepted with a probability of $r$.
\subsection{Subroutine XSUMS }

 This subroutine calculates kinetic and potential sums before the
configuration updates start. Since calculation of the kinetic and potential
sums is a costly operation, after every update we calculate the {\em shift} in the sums.

\subsection{Subroutine ACTION }

This subroutine calculates the action using known values of kinetic and
potential sums. The action is stored in a file to monitor the termalization. ( See Fig.~\ref{action} ).

\subsection{Subroutine UPDSUM }

Since calculation of the kinetic and potential sums is a costly operation,
after every update we calculate the {\em shift} in the sums. Using this
shift sums are updated.

\subsection{Function XDERIV }

This subroutine calculates the derivative operator $S'[Z]$
Eq.~(\ref{groundstate}) which gives the mass of the bound state.

\subsection{Function DELTA, DELTAP }

These subroutine calculate, respectively, the interaction kernel
Eq.~(\ref{kernel.phi3}) and its time derivative.

\subsection{Function DLARAN }

This is a random number generator obtained from LAPACK package at
Netlib.~\cite{random} DLARAN returns a random real number from a
uniform (0,1) distribution. In the actual implementation of the program
we have used a Numerical Recipes random number generator (ran2). However for
copyright reasons here we provide this alternative random number generator.

\subsection{Functions BESK0, BESK1, KZEONE }

BESK0 and BESK1 are modified bessel functions $K_0(x)$ and $K_1(x)$ which
are needed in calculation of the interaction kernel and its derivative.
BESKO and BESK1 call KZEONE subroutine~\cite{kzeone}. KZEONE subroutine
returns real and imaginary parts of $e^xK_0(x)$ and $e^xK_1(x)$. The KZEONE
subroutine is considerably slower than the Numerical Recipes subroutines
for modified bessel functions. For copyright reasons we provide KZEONE rather
than the Numerical Recipes subroutines for the modified bessel functions.

\section{Conclusions}

In this paper, using the Feynman-Schwinger representation, we have presented
an algorithm that calculates 1,2,3 body masses and distribution probabilities
in the quenched approximation for $\chi^2\phi$ theory in 3+1 dimension. The
FSR approach provides an efficient method to calculate nonperturbative
propagators. In this work we have presented results of applications to the
1, 2 and 3 body states. A detailed comparison of quenched bound state results
of the FSR approach with the bound state equation predictions is under study
and will be presented in a separate physics article~\cite{SAVKLI3}. It is hoped that,
through comparison, this simple and rigorous nonperturbative method will
enhance our understanding of various nonperturbative bound state models and
approximations.

\centerline{\bf Acknowledgements}
We are grateful to F. Gross, and J. Tjon for discussions. The support
of the DOE through grant No. DE-FG02-97ER41032 is gratefully acknowledged.
The Thomas Jefferson National Accelerator Facility is gratefully acknowledged
for warm hospitality and for providing computer resources.

\begin{figure}
\begin{center}
\mbox{
   \epsfxsize=3.0in
\epsffile{trajectory2.eps}
}
\end{center}
\caption{A sample trajectory of each particle along with various interactions
are shown. Except the matter loops all self energy, exchange energy and vertex
dressings are included. }
\label{trajectory}
\end{figure}

\begin{figure}[t,h,b]
\begin{center}
\mbox{
   \epsfxsize=5.0in
\epsfbox{sdist.eps}
}
\end{center}
\caption{The sample distribution of Feynman parameter s is shown for two different coupling strengths. The peak of the distribution moves from the
classical value $T/2m$ as the coupling strength is increased.}
\label{sdist}
\end{figure}

\begin{figure}[t,h,b]
\begin{center}
\mbox{
   \epsfxsize=5.0in
\epsfbox{cvsg2.eps}
}
\end{center}
\caption{The dependence of the peak of the s-distribution on the coupling
strength is shown. The peak location is given by $s_0=C T/2m$. Beyond the
critical coupling strenght of $g^2=31 {\rm GeV}^2$ a self consistent
determination of $C$ is not possible. Therefore beyond the critical coupling strength 1-body mass becomes unstable.}
\label{speak}
\end{figure}

\begin{figure}[t,h,b]
\begin{center}
\mbox{
   \epsfxsize=5.0in
\epsfbox{action.eps}
}
\end{center}
\caption{The termalization for two different initial configurations is shown.
Irrespective of the initial conditions the action approaches to an asymptotic
limit. The first 1000 updates are ignored.   }
\label{termalize}
\end{figure}

\begin{figure}[t,h,b]
\begin{center}
\mbox{
   \epsfxsize=5.0in
\epsfbox{correlation.eps}
}
\end{center}
\caption{Here we present the correlation function for the 1-body simulation.
The number of updates necessary for the correlation to vanish is around
$n=1000$. The typical number of updates performed in our simulations, which is
around 500000, is well above the correlation length, thereby insuring that
statistically uncorrelated configurations are sampled.}
\label{correlation}
\end{figure}

\begin{figure}[thb]
\begin{center}
\mbox{
   \epsfxsize=5.0in
\epsfbox{mvsg2.phi3.1b.eps}
}
\end{center}
\caption{The coupling constant dependence of the 1-body dressed mass is
shown. The asymptotic time value $T$ used to obtain these mass values
increase as $g$ increases. While at $g^2=0$ GeV$^2$ $mT=35$ is sufficient, at
 $g^2=31$
GeV$^2$ $mT=45$ is needed. The peak of the s distribution was self
consistently determined. Beyond the critical coupling strength of $g^2=31$
 ${\rm GeV}^2$ the 1-body mass becomes unstable.}
\label{mvsg2.1b}
\end{figure}

\begin{figure}[thb]
\begin{center}
\mbox{
   \epsfxsize=5.0in
\epsfbox{mvsg2.phi3.2b.eps}
}
\end{center}
\caption{The coupling constant dependence of the 2-body bound state mass is
shown. Beyond the critical coupling strength of $g^2=100$ GeV$^2$ the 2-body
mass becomes unstable. }
\label{mvsg2.2b}
\end{figure}

\begin{figure}[t,h,b]
\begin{center}
\mbox{
   \epsfxsize=2.6in
\epsfbox{surface.2b.eps}
}
\end{center}
\caption{The 2-body probability distribution when the 1st particles is at
the origin. The vanishing of probability at the origin is due to the phase
space factor Eq.~(\ref{phase}).}
\label{rdist.surf.2b}
\end{figure}

\begin{figure}[t,h,b]
\begin{center}
\mbox{
   \epsfxsize=5.0in
\epsfbox{rdist.2b.eps}
}
\end{center}
\caption{The radial probability distribution for the 2-body bound state is
shown.
}
\label{rdist.2b}
\end{figure}

\begin{figure}[t,h,b]
\begin{center}
\mbox{
   \epsfxsize=5.5in
\epsfbox{surface.3b.all.color.eps}
}
\end{center}
\caption{Evolution of the probability distribution for the 3rd particle is
shown as the distance between the two fixed particles is increased. When the
fixed particles are very close to each other the third particle sees them as a
point particle (the upper left plot). As the fixed particles are separated
from each other the third particle starts penetrating between them (2nd and 3rd plots), and as the two fixed particles are maximally separated the third particle spends most of its time in between the two fixed particles (the lower
right plot).
  }
\label{rdist.surf.3b}
\end{figure}

\begin{figure}[t,h,b]
\begin{center}
\mbox{
   \epsfxsize=2.0in
\epsfbox{surface.rad.eps}
}
\end{center}
\caption{The radial probability distribution for the 3-body bound state shown
in Fig.~\ref{rdist.surf.3b} includes the phase space factor represented by
the ring in this figure. Distances $r_{13}$, and $r_{23}$ are fixed on the
ring and each point on the ring contribute to the probability distribution shown in Fig.~\ref{rdist.surf.3b}.  }
\label{ring.3b}
\end{figure}

\begin{figure}[t,h,b]
\begin{center}
\mbox{
   \epsfxsize=5.0in
\epsfbox{rdist.3b.eps}
}
\end{center}
\caption{The radial {\em two-body} probability distribution $P_{12}$ for the
3-body bound state is shown. This distribution is obtained by integrating out
the location of the 3rd particle.}
\label{rdist.3b}
\end{figure}

\normalsize

redpajama_set_name: RedPajamaArXiv


Tonight will be "Merk Human Scholarship Night" when the Carson Senators host the Wooster Colts for a double header.
The two teams, now locked in a second-place tie in the Sierra League race, begin the first game at 5 p.m. at Ron McNutt Field. The second game is scheduled for an 8 p.m. start.
Proceeds from the concessions, barbecue and a 50-50 raffle will go toward the newly established Merk Human Scholarship, named in honor of Carson High's long-time fan who passed away in December. The scholarship will be presented to a Carson senior at the team's final regular season home game against Reno on May 2.
Memorial contributions may be made to the Merk Human Baseball Scholarship, c/o Carson High School, 1111 N. Saliman Road, Carson City 89701.


text:
Q: a function for creating shortname style variables in PHP I'm just learning PHP, and I'm sure I'm not the first person to try something like this, but maybe because I didn't know what to call it, I couldn't find any other examples or questions on here or from a search on google.
I wanted to create a function which takes two parameters and uses them to create all the short style variables I'll be using later in my script.
My problem is where normally the syntax to create a short variable is something like:
    $var = $_METHOD['var'];

but I'm trying to do this using variables and don't know how to get the syntax right. Here's my code:
<?php
session_start();

function shortnames($some_vars, $type) {
    for ($i = 0; $i<(count($some_vars)); $i++) {
        $$some_vars[$i] = $_$type['$some_vars[$i]'];
        echo $$some_vars[$i].' = '.$some_vars[$i].'<br />';
    }
}

$post_vars = array(lastname,firstname,payment);
$session_vars = array(sessiontxt,province,city,venue,regfee);

shortnames($session_vars,session);
shortnames($post_vars,post);
?>

Thanks for helping a beginner!!

redpajama_set_name: RedPajamaStackExchange


text:
Our Catalog Christian Books & Bibles Bible Study & Reference Dictionaries & Encyclopedias
Seabrook's Bible Dictionary of Traditional and Mystical Christian Doctrines
Free Shipping Included! Seabrook's Bible Dictionary of Traditional and Mystical Christian Doctrines by Sea Raven Press at Translate This Website. Hurry! Limited time offer. Offer valid only while supplies last. Why are there scores of confusing, mysterious, and even seemingly contradictory scriptures in the Bible? Why does Jesus appear so differently in each of the four Gospels? Why does he continually insist that our focus should be on God, not on him? Why do Mark and John gloss over the Nativity, the world-altering event that justifies all that comes afterward? Why does Paul make no mention of the empty tomb, the very cornerstone of the mainstream Christian Faith? Why does Jesus never use the word
Why are there scores of confusing, mysterious, and even seemingly contradictory scriptures in the Bible? Why does Jesus appear so differently in each of the four Gospels? Why does he continually insist that our focus should be on God, not on him? Why do Mark and John gloss over the Nativity, the world-altering event that justifies all that comes afterward? Why does Paul make no mention of the empty tomb, the very cornerstone of the mainstream Christian Faith? Why does Jesus never use the word "atonement"? Why is he said to have been born in a town called the "House of Bread," and why is he shown growing up in Nazareth, a city that did not exist in the 1st Century A.D.? If there is only one Christ why did Paul say "Christ is in all," and if there is only one God why did Jesus say that we are all gods? What do the mystical Essenes and Gnostics have to do with the original Christian Church, and why were their names purposefully left out of the Bible? Why did Paul declare that he preached "the hidden wisdom of God in a mystery"? Why did Jesus acknowledge that he taught "the mysteries of the Kingdom of God" openly to an inner secret circle of initiates, but parabolically to the general public? What do the Cana Wedding, the Eucharist, the Logos, the Tree of Life, the Serpent, the Virgin Birth, the Resurrection, the Holy Trinity, the Exodus, original sin, Golgotha, the Devil, Noah's ark, Melchizedek, the Son of Man, and the Upper Room, all have in common? Why are such Bible stories and elements as the Fall of Man, the Great Flood, the Virgin-Mother, walking on water, the Three Wise Men, and the crucifixion and resurrection of the Son of God found in countless pre-Christian religions and myths all around the world? You are not likely to get the answers to these questions from any mainstream Church, but you will find them in Seabrook's Bible Dictionary of Traditional and Mystical Christian Doctrines, by Bible authority, spiritual teacher, and award-winning historian Lochlainn Seabrook. This one-of-a-kind, easy to use, 300,000 word reference provides a detailed yet clear examination of the Bible as seen through the eyes of Christian mysticism. By comparing both the outer (exoteric) meanings and the inner (esoteric) meanings of the many sometimes strange and bewildering figures, stories, themes, symbols, words, and allegories in the Good Book, the author provides the missing key to understanding its most cryptic teachings. This illustrated introductory work, steeped in intriguing historical references, seldom-discussed scriptures, and forgotten arcane doctrines, will appeal to anyone - Christian or non-Christian, believer or non-believer - with an open inquiring mind, and a desire to gain a deeper more complete understanding of the Bible; one that goes far beyond what is typically taught by the mainline established Church. The result of decades of study and research, and with nearly 5,000 endnotes and a 1,200 book bibliography, Seabrook's Bible Dictionary is sure to enlighten, educate, and fascinate. Whether you are a Liberal Christian or a Conservative Christian, this landmark volume is a must-have for both serious Bible students and casual readers, as well as for preachers, theologians, scholars, and the clergy. Available in paperback and hardcover. "An uplifting and highly informative celebration of all that it means to be Christian, based on the long suppressed mystical teachings of Jesus and his first followers." - The Publisher. Colonel Lochlainn Seabrook is an award-winning historian and Bible authority, and the author of over 50 books that have introduced hundreds of thousands to the hidden truths contained within the Bible. His other titles include: Jesus and the Gospel of Q, and Christ is All and in All.
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text:
NHL All Star Game
Ranking the Best NHL All-Star Game Performances from the Last Decade
Tom Urtz Jr.@@TomUrtzJrTwitter LogoContributor IJanuary 23, 2015
Jamie Sabau/Getty Images
Over the last decade, there have been some amazing All-Star Games played, and each had some memorable performances. There was Alex Kovalev starring in Montreal, Daniel Alfredsson playing in his final All-Star Game in Ottawa and much more.
There are players who went above and beyond during the last 10 years, and here are the 12 best individual performances from 2004 to the present.
12. Henrik Sedin (2012)
Stats: 1 Goal, 2 Assists
The 2012 All-Star Game is going to be featured here a few times, because there were a number of solid performances. During this game, the Sedin twins were paired on Team Alfredsson, and it was Henrik who stole the show.
The Vancouver Canucks captain tallied a goal and two assists, and both Daniel Sedin and Daniel Alfredsson accompanied him on the stat sheet twice.
11. Marian Hossa (2012)
Marian Hossa tallied the same amount of points as Henrik Sedin at the 2012 All-Star Game, except he was a member of Team Chara. The Slovak Sniper was able to set up MVP Marian Gaborik twice. Hossa was also able to assist fellow countryman Zdeno Chara, so it ended up being an evening that featured several Slovak stars.
Hossa is a five-time All-Star, and you will hear about his best game a couple of slides later.
10. Daniel Alfredsson (2012)
Stats: 2 Goals, 1 Assist
If Team Alfredsson had won the 2012 All-Star Game, Daniel would have taken home MVP honors. In his home rink, Alfredsson scored two goals and an assist, including an unassisted goal.
The Ottawa Senators' long-time captain was able to make the most of his final All-Star Game, and it certainly was a night to remember.
9. Eric Staal (2008)
Andre Ringuette/Getty Images
Stats: 2 Goals, 1 Assist, MVP
Eric Staal was named MVP of the 2008 All-Star Game held in Atlanta, and the captain of the Carolina Hurricanes had quite a performance.
Staal recorded a goal and an assist through the first two periods of the game, and he scored the game-tying goal in the third period, which changed the pace of the game. A goal by Marc Savard sealed the deal late in the third, and Staal had a hand in setting the final play up.
It is easy for players to get caught up in the fanfare of All-Star Games, but Staal was on point the entire night.
8. Martin St. Louis (2009)
Martin St. Louis is a prolific scorer who has been a frequent participant at the All-Star Game. Back in 2009, St. Louis played for the Eastern Conference All-Stars, and he recorded two goals and an assist.
St. Louis was involved in two goals that took place 50 seconds apart, and his hot play allowed the East to get out to a big lead early on in the game.
In addition to that, St. Louis impressed during the Skills Competition, so it was a great weekend for him overall.
7. Rick Nash (2008)
Stats: 3 Goals
In the video above, James Duthie of TSN pointed out that "Slick" Rick Nash has a knack for coming up big at the All-Star Game, so look for him to turn heads on Sunday. Back in 2008, Nash was a menace for the Western Conference, and he found the back of the net three times.
Nash came close to scoring a fourth goal that would have made Joe Thornton proud, but it was never meant to be. You would think a hat trick would be higher on this list, but Nash had an even better performance at the 2007 All-Star Game.
6. Marian Hossa (2007)
Dave Sandford/Getty Images
Stats: 4 Assists
The 2007 All-Star Game was a landslide because of a very dynamic Western Conference offense, but the Eastern Conference didn't take the onslaught lying down. After trailing heavily for most of the game, Hossa was involved with three third-period goals that almost helped the East get back into the game.
Throughout the evening, Hossa's underrated mitts were on display, and he would have had a shot at taking home the MVP award if his team ended up winning the game.
Ronald Martinez/Getty Images
Stats: 2 Goals, 2 Assists
As we found out in Slide No. 6, Rick Nash is money at the All-Star Game. In 2007, the power forward made magic with Hall of Fame pivot Joe Sakic, as the duo were involved in four goals together.
Sakic was able to hold onto the puck for the majority of the night, and he found ways to distribute it to a skilled sniper like Nash whenever he wanted to.
Nash has a knack for coming up big during All-Star weekend, but 2007 was by far his greatest performance to date.
4. Joe Sakic (2007)
As fantastic as Rick Nash was at the 2007 All-Star Game, Joe Sakic was even better. The legendary center went out with a bang in his final All-Star Game, as he recorded four assists. The puck was like an egg on his stick all night long, cradled with the utmost care.
Burnaby Joe's efforts were a big reason behind the Western Conference's dominance in that game, and the captain delivered one of the best All-Star Game performances of his storied career.
Stats: 3 Goals, MVP
The final All-Star Game before the lockout took place was held in St. Paul, and it was a lopsided game in which the Western Conference lost 6-4. A couple of different players for the East—including Mark Messier, Daniel Alfredsson, Mats Sundin and Gary Roberts—dominated the night, but Sakic ultimately came out on top.
Sakic gets the nod here because he scored three of the West's four goals and was the MVP for being the best individual player on the ice. Markus Naslund did record three assists that night, but none of them were especially memorable.
2. Marian Gaborik (2012)
Marian Gaborik had an amazing evening at the 2012 All-Star Game as a representative of the New York Rangers. It was a season in which Gaborik was able to stay healthy and put his full arsenal of skills on display.
The speedy winger found the net three times, and he added a helper for good measure. Gaborik ran away with the MVP honors, and it was an electric night for a magnetic player.
1. Daniel Briere (2007)
Al Messerschmidt/Getty Images
Stats: 1 Goal, 4 Assists, MVP
Daniel Briere tops the list because of his amazing and unexpected offensive explosion at the 2007 All-Star Game.
Over the last decade, there have been skilled scorers such as Alex Ovechkin, Evgeni Malkin, Steven Stamkos and Rick Nash who have appeared in an All-Star Game, but none of them were able to score five points in a single showing.
Briere was the main man at the 2007 game, and his goal and four assists enabled him to take home MVP honors.
Stats via Wikipedia's NHL All-Star Game section.


text:
Mahey, the boy-wonder, finds home at FC Porto
by Rossoneris Selecao · February 12, 2021
So I wandered about one afternoon at Aboabu, a suburb of Tamale. At sundown, I was around the Metro Mass Station and decided to go and watch football at the cluster of fields in the famous forest nearby. It's a hub of football in the mornings and afternoons that has birthed many footballers, past and present.
By sheer coincidence, the first piece of action I saw set my mind into thought and dazed my eyes. There was a tall, lanky, barefooted kid who was head and shoulders above everyone else, with a gait akin to that of Argentina legend Juan Roman Riquelme.
This kid readied himself for a long ball and as it beckoned, with an opponent in pursuit, he chested the ball into space with the swagger of a master, and then rolled it with his right sole as it touched the ground. It was an orgasmic flash of brilliance completely unscripted or foreseen. I fell in love, at first sight.
My curiosity led to enquiries and Abdul Moomin Mohammed, popularly known as Mahey became a case study. A player of Real Republicans, coached by the legendary Alhassan Dawuo, my craze got me closer to the iconic Colts club just to watch this boy in matches. Mahey never ceased to amaze.
Information would spread about a young boy with incredible talent. He exuded brainwork that belied his age. Gifted with technique, Mahey boasts of impeccable ball control, accurate passing, shot power and the knack for hustling for the ball. As a deep lying midfielder, he dictates the pace of play with admiration and is capable of threading through the final pass with style.
Mahey's talent took him to Charity FC, a Division Two side at Kaneshie in Accra. He would spend two seasons there, a period that saw them take part in numerous tournaments in Accra and Kumasi. In doing this, he would impress scouts, local and foreign, with his ability on the ball. The passage of time made it clear that his days in Ghana were numbered.
Portuguese giants FC Porto were nosing around. They took notice and never looked back. An invitation for trials came in earnest but COVID travel restrictions had other ideas. Upon easing of restrictions, Mahey jetted to Portugal to kickstart what should be a brilliant career.
After training with the Porto U-19s for some time, and playing in friendlies, the inevitable happened. He has been offered a six-month loan deal with option to buy. Haven put pen to paper, Mahey knows his work is cut out for him. A remarkable run of form, laced with eye-catching performances is all he craves. To make a loan deal permanent and possibly break into the first team, his feet must do their job.
No one who has watched this youngster will doubt him. He has got tremendous talent to succeed. Talent alone though, is not always enough. It needs associates in the form of prayer, hard work, determination, amongst others. Perhaps, soon, the next Thomas Partey will be on the horizon. Mahey cites the Arsenal star as his role model, alongside Leicester City's Nigerian international Wilfred Ndidi. Go for gold, Mahey.
Yours in the beautiful game
Tags: MaheyThomas Partey
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I know I can work well with clients from Ontario online through cybercounselling or in-person in Zürich.


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