Towse: More pics with the new camera.
and asked, What a gorgeous shot! Did you "do" anything to it?
That's "as taken." Must be the new camera! I use Picasa for the quick "straighten that horizon" work that I sometimes need because of sloppiness or the astigmatism. You can also sharpen, highlight, crank up the saturation, crop, &c.
If you spin through a Picasa "library," you can tell whenever you've done anything because Picasa shows you a quick look at the original and then says, "refining."
I doublechecked and this shot has no "refining" at all.
The camera's a gem. My first digital camera -- purchased June 2004 -- was a simple camera to see if I liked shooting digital. This Nikon CoolPix 5600 is more sophisticated, more pixels, optical zoom in additional to digital zoom, more tools.
A nice feature is that if you're shooting, f'rex, in "sunset" mode, which makes the shutter speed slower than normal and (just suppose) you're cranked up to 3x optical zoom, and your hand jiggers a bit, the camera very politely sez, "Hey, you up screwed that one. It's really blurred. Do you really want me to save it?"
Here's a sunset shot from yesterday. The sun is setting behind me, to the west, and threw some beautiful color on the clouds to the southeast.
And the Abe (which you can see anchored to the south of the Bay Bridge in the sunset picture above) left this morning. The sailors had a liberty weekend. (How many had tickets to see the Stones at SBC Park?) Throughout the visit, there was no news, no protests, no nothing. Here's a picture as it left, Yerba Buena to your right. Treasure Island and the Admin Building to the left. Berkeley (Hi, Harry! Hi, Don!) in the background.
We were at a neighbor's Canadian (i.e. "for no good reason with insufficient notice") party on Saturday. Despite the advice of another neighbor (former bartender) to "drink only wine, beer, brown, clear," I had far too many pale green minty shots of something and spent yesterday wishing I hadn't.
At the neighbor party, I met a guy who is a neighbor from the other side of Coit Tower. Mikkel Aaland is a photographer-type who writes about digital photography. We'd been talking about my old camera dying and the search for the new one.
"Which camera?" (meaning the old one) he asked.
"Oh. So, what did you buy?"
Yay. Always nice to have your choices affirmed by someone who knows more than you do.
UV sed, New cameras are always so much fun.


Leading heritage photographer Steven Sklifas will present a lecture entitled "Photographic odyssey of the legacy and glory of the Ancient Greek and Hellenistic world", on Thursday 30 March 2017, as a part of the Greek History and Culture Seminars of the Greek Community of Melbourne.
It must be noted that the lecture will take place at the Ithacan Philanthropic Society (Level 2, 329 Elizabeth Street, Melbourne), at 7.00pm, and not at the Greek Centre.
The Ancient Greeks founded and Hellenised hundreds of settlements all around the Mediterranean. Some of these settlements have endured the winds of change and thrived, while some others lay majestic in their ruins and provide a poignant insight to their former glory.
This lecture will take the audience on an informative, insightful, and evocative photographic odyssey to ancient sites found in Greece and to those former Greek settlements throughout the Mediterranean highlighting the greatness, splendour, and enduring legacy of the Ancient Greeks.
Steven Sklifas is independent freelance photographer who has travelled throughout the Mediterranean. He is considered a leading heritage photographer of the region. His images have been extensively published worldwide and have featured in exhibitions, academic and history books and travel magazines and newspapers. His images were included in the exhibition- "Power and Pathos: Bronze Sculpture of the Hellenistic World" which was held at the Getty Museum and National Gallery of Art Washington DC. Steven has also written several travel articles, for Australian newspapers.


text:
Here is a very good interview with M.I.A from the village voice. She talks about the production of her new album, her trips around the world, the perks of not working with big time producers, and where she's at musically. Check it out:
****There's a Timabaland track that I guess is a bonus track on the album in the US, and it's on his album in the UK. It's a great song, but there's a part where he's like, 'Baby girl go to your teepee.' What was that?
Don't ask me! It was kind of funny. I don't like to butt in when that's going on. I just thought it was pretty funny at the time, so I left it. It was kind of funny to meet him and work with him. It was amazing because he's amazing at what he does; he's a legend. But by the time that our paths met, Timbaland had already been Timbaland and done all the cool weird shit. He's sampled babies and cows and things, and I was making tracks sampling chickens. And he was like, "I'm done being cool; I want to work with Celine Dion." And I was like, "So you just want to make Titanic?" And he's like, "Yeah, that's what I want to do." In my career right now, I'm not trying to make Titanic. I want my songs to just be what they are, and I wasn't thinking like that.
So that's what "Jimmy" is about? The journalist?
Well, "Jimmy" the song is a really old Bollywood disco song. It was huge. It's like "Thriller." When I was a kid in Sri Lanka, it meant a lot to me. My mom used to get me to be a professional party buffer. I used to dance a lot as a kid, so people hired me out at birthday parties. That was my theme song. I used to do a performance to "Jimmy." I used to have a cloak and a cardboard guitar, and I'd do this big disco-dancing number and get all the kids to dance, and then they'd pay me and I'd leave. So that song to me is really really personal. And I was in this place, in Liberia, and it was really heavy. I was doing lots of heavy, heavy stuff, not really thinking about romance. And obviously I'd been in this weird relationship before, and I'd come out of it, like "Maybe I should just do this mad trip and go meet this person." And it's just a mash-up of all those things, whatever I was going through that week. I wanted to redo "Jimmy" for a long time. When I was in India, I'd already recorded the strings and everything for it. But I'd never attempted to do "Jimmy" the whole time I was with Switch because it was just one of those songs; I had to be drunk enough to be that disco. It all came together that week.****
Thannks to TimboFan for the link.
Posted by J Boogie at 10:39 AM
Labels: M.I.A.

redpajama_set_name: RedPajamaCommonCrawl


text:
<!DOCTYPE html>

    <meta charset="utf-8">
    <meta name="viewport" content="width=device-width, initial-scale=1.0">
    <meta name="generator" content="rustdoc">
    <meta name="description" content="API documentation for the Rust `ser` mod in crate `serde`.">
    <meta name="keywords" content="rust, rustlang, rust-lang, ser">

    <title>serde::ser - Rust</title>

    <link rel="stylesheet" type="text/css" href="../../normalize.css">
    <link rel="stylesheet" type="text/css" href="../../rustdoc.css">
    <link rel="stylesheet" type="text/css" href="../../main.css">

serde

        <form class="search-form js-only">

                <input class="search-input" name="search"
                       autocomplete="off"
                       placeholder="Click or press 'S' to search, '?' for more options…"
                       type="search">

        </form>

Module serde::<wbr>ser

                       [−]

               [src]

Generic data structure serialization framework.

The two most important traits in this module are Serialize and
Serializer.

A type that implements Serialize is a data structure that can be
serialized to any data format supported by Serde, and conversely

A type that implements Serializer is a data format that can
serialize any data structure supported by Serde.

The Serialize trait

Serde provides Serialize implementations for many Rust primitive and
standard library types. The complete list is below. All of these can be
serialized using Serde out of the box.

Additionally, Serde provides a procedural macro called serde_derive to
automatically generate Serialize implementations for structs and enums
in your program. See the codegen section of the manual for how to use
this.

In rare cases it may be necessary to implement Serialize manually for
some type in your program. See the Implementing Serialize section of the
manual for more about this.

Third-party crates may provide Serialize implementations for types that
they expose. For example the linked-hash-map crate provides a
LinkedHashMap<K, V> type that is serializable by Serde because the crate
provides an implementation of Serialize for it.

The Serializer trait

Serializer implementations are provided by third-party crates, for
example serde_json, serde_yaml and bincode.

A partial list of well-maintained formats is given on the Serde
website.

Implementations of Serialize provided by Serde

Primitive types:

bool

i8, i16, i32, i64, isize

u8, u16, u32, u64, usize

f32, f64

char

str

&T and &mut T

Compound types:

[T]

[T; 0] through [T; 32]

tuples up to size 16

Common standard library types:

String

Option<T>

Result<T, E>

PhantomData<T>

Wrapper types:

Box<T>

Rc<T>

Arc<T>

Cow<'a, T>

Cell<T>

RefCell<T>

Mutex<T>

RwLock<T>

Collection types:

BTreeMap<K, V>

BTreeSet<T>

BinaryHeap<T>

HashMap<K, V, H>

HashSet<T, H>

LinkedList<T>

VecDeque<T>

Vec<T>

EnumSet<T> (unstable)

FFI types:

CStr

CString

OsStr

OsString

Miscellaneous standard library types:

Duration

Path

PathBuf

Range<T>

NonZero<T> (unstable)

Net types:

IpAddr

Ipv4Addr

Ipv6Addr

SocketAddr

SocketAddrV4

SocketAddrV6

Structs

                           Impossible

Helper type for implementing a Serializer that does not support
serializing one of the compound types.

Traits

                           Error

Trait used by Serialize implementations to generically construct
errors belonging to the Serializer against which they are
currently running.

                           Serialize

A data structure that can be serialized into any data format supported
by Serde.

                           SerializeMap

Returned from Serializer::serialize_map.

                           SerializeSeq

Returned from Serializer::serialize_seq.

                           SerializeStruct

Returned from Serializer::serialize_struct.

                           SerializeStructVariant

Returned from Serializer::serialize_struct_variant.

                           SerializeTuple

Returned from Serializer::serialize_tuple.

                           SerializeTupleStruct

Returned from Serializer::serialize_tuple_struct.

                           SerializeTupleVariant

Returned from Serializer::serialize_tuple_variant.

                           Serializer

A data format that can serialize any data structure supported by Serde.

Help

Keyboard Shortcuts

?

Show this help dialog

S

Focus the search field

⇤

Move up in search results

⇥

Move down in search results

⏎

Go to active search result

+

Collapse/expand all sections

Search Tricks

                    Prefix searches with a type followed by a colon (e.g.
                    fn:) to restrict the search to a given type.

                    Accepted types are: fn, mod,
                    struct, enum,
                    trait, type, macro,
                    and const.

                    Search functions by type signature (e.g.
                    vec -> usize or * -> vec)

redpajama_set_name: RedPajamaGithub


Brexitology – Are my eyes really blue?
Logically speaking, the thing that sticks out is that official Britain seems committed to leaving the European Union on March 29, deal or no deal, based solely on a 52% vote in a referendum that is not technically binding. So setting aside the question of whether that is remotely sane, let's assume that this is going to happen no matter what. Let's further accept that the EU deal that was voted down 2-1 tonight is in fact the best deal the UK can get, and the alternative is to leave with no deal. At this point, there's nothing left to argue about. Britain is going to crash out of the EU on March 29.
You can make a case for pulling the plug on Brexit based on the notion that this isn't what people thought they were getting. That's entirely plausible – you could make a good case that a hard no-deal Brexit with all its consequences is far too grave a circumstance to let go on the basis of a single 52% referendum vote. But the deal that's presently on offer can almost certainly not be improved upon. It's not that Theresa May screwed up – her performance has been manifestly disastrous, but that's only marginally on her and mostly on the fact that there is no way to do this well. The Brexiteer fantasy of "everything we want and nothing we don't" is not on offer, and the people fighting on those grounds are out of their mind. That said, there was nothing that said May had to trigger Article 50 before a deal was in place; the March 29 deadline didn't have to be there and the looming cliff was chosen, not imposed.
And if Britain goes off that cliff, that's it. There's no going back. You can't expect to rejoin the EU at some future date with the arrangements that existed previously. Best case scenario is a Norway-type arrangement where you have all the rules and none of the power to shape them. More likely is an obligation to come back with hat in hand and accept full membership, complete with the Euro replacing the pound and no rebates on the common agriculture protocol. But right now, you have to think that No Deal is going to win, simply because that's on autopilot and requires nothing. It would take an affirmative vote to accomplish anything, and nobody can agree on an affirmative path – the deal is unacceptable, bailing out of Brexit altogether is unacceptable (?), so follow the rails until you run off 'em.
I don't think Cold War begins to cover it. This is a Cold Invasion, ongoing for years, of a type that wasn't possible before the advent of the Internet and wasn't conceivable when there were still societal standards around news, truth and the norms of the democratic process. We let the "choose your own reality" types undermine our existence until it only took a social media push to bring the whole edifice to its knees.
The tough bit is learning how to plow through the next day despite a constant fog of existential despair. And the day after that. And the day after that. And while you can do it, you end up having to circumscribe the world around you and narrow your focus and not think of other people or think of the future or think about the bigger issues. Which is what they wanted to begin with. So the question we keep coming back to – if you can't come up with a path to victory, how do you at least stave off defeat without giving them what they want?


Congratulations! You have found the Cyprinidae Forum on Forum Jar. This forum is a place where people who are interested in Cyprinidae come together and discuss about Cyprinidae. Please use the message board below to post anything related to Cyprinidae . If you are interested in other similar forums, please check out the Related Forums section on the right. If you like this forum, please don't forget to tell your friends about Forum Jar.
There are no entries in Cyprinidae forum. Become the first person to post messages in this forum by using the form below!


text:
Home » Private Music Lessons » Brass & Winds
Nancy Ackerman
Nancy Helene Ackerman is a clarinetist, chamber coach, and music educator who lives and works in the Worcester area. She has been a faculty member at the Joy of Music Program (JOMP) since 2008. She also teaches private music lessons at her home studio specializing in clarinet, flute, and saxophone.
Nancy received her B.S. in Music Education from Nazareth College of Rochester, and a M.M. in Woodwind Performance at Boston University. She has studied with Michael Webster, Stanley Gaulke, and while in Rennes, France with Charles Rouault.
Recent performances have included several programs of women composers for the clarinet, and lectures and recitals of the clarinet compositions of Walter Byron Mourant. Nancy also performs frequently as a soloist for worship services throughout Massachusetts.
She enjoys working with her fellow musicians in faculty recitals hosted by the Joy of Music. Programs have included Music of the German Romantics for soprano, clarinet, and piano; music for clarinet, viola, and piano; music for clarinet, violin, and piano; and most recently a program of French composers for flute, clarinet, and piano.
Students of Nancy have participated in both Eastern and Central District Junior and Senior Bands and Orchestras as well as at the Massachusetts All-State Conference, some earning principal positions. After high school, some of her students go on to major or minor in music in college, and many, while pursuing other degree programs, participate in musical organizations offered at their colleges and universities.
As a music educator, Nancy enjoys working with students of all ages and levels, and believes that music and art should be a part of everyone's educational experience. Click here to see Nancy's website: www.westwyndmusic.com
Music Theory Ages: Teen to Adult
Woodwind Ensembles
Clarinet, Flute, Beginning Recorder, Saxophone
MTWThF
Kenji Kikuchi
Kenji Kikuchi, composer, saxophonist and music educator, has appeared as a performer internationally, including Carnegie Hall, the Sydney Opera House and the Montreux Jazz Festival. He has performed with many jazz greats, including Joshua Redman, Richard Davis, Abraham Laboriel, Jr., Greg Hopkins and Joe Hunt. He is an active performer in the style of classical and jazz on not only his primary instrument, saxophone, but also on flute and clarinet.
Mr. Kikuchi is also an accomplished composer of contemporary classical music. He had several of his works premiered, including Overture for Orchestra and Saxophone Concerto by the Quincy Symphony; Marimba Concerto and Prelude for Orchestra by the Melrose Symphony; and Cape Ann Overture by the Cape Ann Symphony. He has also published Astronomy I, II (Finalist, National Flute Association Newly Published Piece, 2002), Quartet No. 2 (Winner, National Flute Association Newly Published Piece, 1998) and Airmail Edition with Falls House Press; and Sonata for Flute and Piano and Piece for Solo Piano with BKJ Publications. His compositions and arrangements have been performed at renowned venues such as Carnegie Hall, Lincoln Center and Boston Symphony Hall.
As a music educator, Mr. Kikuchi has been directing Soul Sauce, the Groton School Jazz Ensemble, for thirteen years, and he provides opportunities to young musicians to learn both performing with harmony in a group and developing their individual voices through jazz music. He joined the Joy of Music faculty in the fall of 2017.
Clarinet, Flute, Saxophone
On Leave
Vlad Vaskevich
Vlad Vaskevich, a clarinet and saxophone performer, music educator, and arranger received his Bachelor of Music in Clarinet from the internationally-known Stolyarsky School of Music for Talented Youth and his Master of Music degree in Clarinet from Odessa State Conservatory, where he studied clarinet performance with Professor Kalio Muhlberg.
While studying classical music, Vlad developed a particular interest in jazz. In the Worcester area, he was one of the ArtsWorcester Jazz Ensemble founders, and his name is included in the Jazz Worcester Real Book and "Worcester Jazz History Tree." Vlad has been professionally performing concerts of popular classical and jazz music throughout New England for many years. At Joy of Music, Vlad has performed multi-genre faculty recitals, consisting of classical music for clarinet for the first half and jazz music for saxophone for the second. His recitals have featured collaborations with such great educators and performers as Wendy Ardizzone, Jerri Sabatini, Rich Ardizzone, Mike Connors, Kallin Johnson, Joe D'Angelo, Thaddeus Bell, and Gerry Wilfong.
An energetic and devoted teacher, Vlad takes great pride in his students' achievements. Every year his students have performed in the Massachusetts Central District and All-State Festival Concerts, some of them as the principal players. His students also participated in the NEC Massachusetts Youth Wind Ensemble, the Boston, Worcester, and Joy of Music Youth Symphony Orchestras. Several of his students are winners of Young Artist Competitions and have performed their solo programs with symphony orchestras in concerts.
Vlad has been a faculty member at the Performing Arts School of Worcester, Clark University, and the John Hopkins University National Center for Talented Youth. Currently, Vlad teaches clarinet and saxophone at the Artists in Residence program at Wachusett Regional School District and the Cape Conservatory (since 2014). He continues to teach at his private studio in Holden. Vlad has been on the Joy of Music faculty since 2006.
Clarinet, Saxophone
Flexible remote


Polycyclic aromatic hydrocarbons (PAHs) are ubiquitous environmental contaminants. Traditionally, much of the research has focused on the carcinogenic potential of specific PAHs, such as benzo(a)pyrene, but recent studies using sensitive fish models have shown that exposure to PAHs alters normal fish development. Some PAHs can induce a teratogenic phenotype similar to that caused by planar halogenated aromatic hydrocarbons, such as dioxin. Consequently, mechanism of action is often equated between the two classes of compounds. Unlike dioxins, however, the developmental toxicity of PAH mixtures is not necessarily additive. This is likely related to their multiple mechanisms of toxicity and their rapid biotransformation by CYP1 enzymes to metabolites with a wide array of structures and potential toxicities. This has important implications for risk assessment and management as the current approach for complex mixtures of PAHs usually assumes concentration addition. In this review we discuss our current knowledge of teratogenicity caused by single PAH compounds and by mixtures and the importance of these latest findings for adequately assessing risk of PAHs to humans and wildlife. Throughout, we place particular emphasis on research on the early life stages of fish, which has proven to be a sensitive and rapid developmental model to elucidate effects of hydrocarbon mixtures.


text:
Q: Machine dependent _write failures with EINVAL error code This has some lengthy background before the actual question, however, it bears some explaining to hopefully weed out some red herrings.
Our application, developed in Microsoft Visual C++ (2005), uses a 3rd party library (whose source code we luckily happen to have) to export a compressed file used in another 3rd party application.  The library is responsible for creating the exported file, managing the data and compression, and generally handling all errors.  Recently, we began getting feedback that on certain machines, our application would crash during writes to the file.  Based on some initial exploration, we were able to determine the following:

*

*The crashes happened on a variety of hardware setups and Operating Systems (although our customers are restricted to XP / 2000)

*The crashes would always happen on the same set of data; however they would not occur on all sets of data

*For a set of data that caused a crash, the crash is not reproducible on all machines, even with similar characteristics, i.e., operating system, amount of RAM, etc.

*The bug would only manifest itself when the application was run in the installation directory - not when built from Visual Studio, run in debug mode, or even run in other directories that the user had access to

*The issue occurs whether the file is being constructed on a local or a mapped drive

Upon investigating the problem, we found the issue to be in the following block of code (slightly modified to remove some macros):
 while (size>0) {
    do {
        nbytes = _write(file->fd, buf, size);
    } while (-1==nbytes && EINTR==errno);
    if (-1==nbytes) /* error */
        throw("file write failed")
    assert(nbytes>0);
    assert((size_t)nbytes<=size);
    size -= (size_t)nbytes;
    addr += (haddr_t)nbytes;
    buf = (const char*)buf + nbytes;
}

Specifically, the _write is returning error code 22, or EINVAL.  According to MSDN, _write returning EINVAL implies that the buffer (buf in this case) is a null pointer.  Some simple checks however around this function verified that this was not the case in any calls made to it.
We do, however, call this method with some very large sets of data - upwards of 250MB in a single call, depending on the input data.  When we imposed an artificial limit on the amount of data that went to this method, we appear to have resolved the issue.  This, however, smacks of a code fix for a problem that is machine dependent / permissions dependent / dependent on the phase of the moon.  So now the questions:

*

*Is anyone aware of a limit on the amount of data _write can handle in a single call?  Or - barring _write - any file I/O command support by Visual C++?

*Since this does not occur on all machines - or even on every call that is a sufficient size (one call with 250 MB will work, another call will not) - is anyone aware of user, machine, group policy settings, or folder permissions that would affect this?

UPDATE:
A few other points, from the posts so far:

*

*We do handle the cases where the large buffer allocation fails.  For performance reasons in the 3rd party application that reads the file we're creating, we want to write all the data out in one big block (although given this error, it may not be possible)

*We have checked the initial value of size in the routine above, and it is the same as the size of the buffer that was allocated.  Also, when the EINVAL error code is raised, size is equal to 0, and buf is not a null pointer - which makes me think that this isn't the cause of the problem.

Another Update:
An example of a failure is below with some handy printfs in the code sample above.
     while (size>0) {
    if (NULL == buf)
    {
        printf("Buffer is null\n");
    }
    do {
        nbytes = _write(file->fd, buf, size);
    } while (-1==nbytes && EINTR==errno);
    if (-1==nbytes) /* error */
    {
        if (NULL == buf)
        {
            printf("Buffer is null post write\n");
        }
        printf("Error number: %d\n", errno);
        printf("Buffer address: %d\n", &buf);
        printf("Size: %d\n", size);
        throw("file write failed")
    }
    assert(nbytes>0);
    assert((size_t)nbytes<=size);
    size -= (size_t)nbytes;
    addr += (haddr_t)nbytes;
    buf = (const char*)buf + nbytes;
}

On a failure, this will print out:
Error number: 22
Buffer address: 1194824
Size: 89702400

Note that no bytes were successfully written and that the buffer has a valid address (and no NULL pointer checks were triggered, pre or post _write)
LAST UPDATE
Unfortunately, we were overcome by events and were not able to conclusively solve this.  We were able to find some interesting (and maybe even disturbing) facts.
1. The errors only occurred on machines with slower write times on their hard disks.  Two PCs, with the exact same hardware specs, but with different RAID configurations (RAID 0 versus RAID 1) would have different results.  The RAID 0 would process the data correctly; the RAID 1 would fail.  Similarly, older PCs with slower hard drives would also fail; newers PCs with faster hard drives - but similar processors / memory - would work.
2. The write size mattered.  When we limited the amount of data passed to _write to be 64 MB, all but one file succeeded.  When we limited it to 32 MB, all the files succeeded.  We took a performance hit in the library we were using - which was a limitation of that library and independent of _write or the problem we were seeing - but it was our only "software" fix.
Unfortunately, I never got a good answer (and we were about to call Microsoft on this, but we had to get business to sign off on the expense of a tech support call) as to why the EINVAL was being returned in the first place.  It isn't - from what we were able to find - documented anywhere in the C library API.
If anyone does find a good answer for this, please post it on here and I'll mark it as the answer.  I'd love to get a conclusion for this saga, even if it no longer directly applies to me.

A: We had a very similar problem which we managed to reproduce quite easily. We first compiled the following program:
#include <stdlib.h>
#include <stdio.h>
#include <io.h>
#include <sys/stat.h>
#include <fcntl.h>

int main(int argc, char *argv[])
{ int len = 70000000;
  int handle= creat(argv[1], S_IWRITE | S_IREAD);
  setmode (handle, _O_BINARY);
  void *buf = malloc(len);
  int byteswritten = write(handle, buf, len);
  if (byteswritten == len)
    printf("Write successful.\n");
  else
    printf("Write failed.\n");
  close(handle);
  return 0;
}

Now, let's say you are working on the computer mycomputer and that C:\inbox maps to a shared folder \\mycomputer\inbox. Then the observe the following effect:
C:\>a.exe C:\inbox\x
Write successful.

C:\>a.exe \\mycomputer\inbox\x
Write failed.

Note that if len is changed to 60000000, there is no problem...
Based on this web page support.microsoft.com/kb/899149, we think it is a "limitation of the operating system" (the same effect has been observed with fwrite). Our work around is to try to cut the write in 63 MB pieces if it fails. This problem has apparently been corrected on Windows Vista.
I hope this helps!
Simon

A: Did you look at the implementation of _write() in the CRT (C runtime) source that was installed with Visual Studio (C:\Program Files\Microsoft Visual Studio 8\VC\crt\src\write.c)?
There are at least two conditions that cause _write() to set errno to EINVAL:

*

*buffer is NULL, as you mentioned.

*count parameter is odd when the file is opened in text mode in UTF-16 format (or UTF-8? the comments don't match the code). Is this a text or binary file? If it's text, does it have a byte order mark?

*Perhaps another function that _write() calls also sets errno to EINVAL?

If you can reliably reproduce this problem, you should be able to narrow down the source of the error by putting breakpoints in the parts of the CRT source that set the error code. It also appears that the debug version of the CRT is capable of asserting when the error occurs, but it might require tweaking some options (I haven't tried it).

A: According to http://msdn.microsoft.com/en-us/library/1570wh78(v=VS.90).aspx
errno can take the values:
- EBADF
- ENOSPC
- EINVAL.

There is not EINTR on windows. Random system interrupts cause this error and are not caught by the test while (-1==nbytes && EINTR==errno);

A: Two thoughts come to mind..  Either you are walking past the end of the buffer, and trying to write that data out, or the allocation of the buffer failed.  Problems that, in debug mode, will not be as visible as they are in release mode.
It's probably a bad idea to allocate 250 meg of memory anyways.  You'd do better to allocate a fixed size buffer, and do your writing in chunks.
Have you looked for things like Virus Scanners that might have a hold on the file in between your write operations, thus making the write fail?
I know of no limit to the amount of data you can pass to write in a single call, unless (like I said), you are writing data (as part of the buffer) that does not belong to you...
Since most of these functions wrap the Kernel call WriteFile(), (Or NtWriteFile()), there COULD be the condition that there isn't enough Kernel memory to handle the buffer to write.  But, THAT I'm not certain of, since I don't know WHEN exactly the code makes the jump from UM to KM.
Don't know if any of this will help, but hope it does...
If you can provide any more details, please do.  Sometimes just telling someone about the problem will trigger your brain to go "Wait a minute!", and you'll figure it out.  heh..

A: You could be trashing your own stack by accidentally misusing a pointer somewhere else - if you can find a repro machine, try running your app under Application Verifier with all the memory checks turned on

redpajama_set_name: RedPajamaStackExchange


text:
\section{Introduction} Bound states in quantum field theories are usually considered in
the c.m. system, however many practical applications need the corresponding
wave functions in the arbitrarily moving system, e.g. in formfactors, reaction
etc.

On  the theoretical side the rules of the special relativity can predict the
frame dependence for the global characteristics,  such as the total energy.
However, for the internal characteristics  e.g.  wave functions, the general
theory is still unable to give answers, since the frame dependence of the full
dynamics includes the interaction term  \cite{1}.

A part of this difficulty is connected to the standard formalism of
relativistic bound state equations, based on the Bethe-Salpeter integral
equations, which is a complicated and not always  a rigorous instrument
(problems of the relative time, spurious solutions and difficulty to implement
nonperturbative effects).

The study of boost effects in this framework was done in \cite{2,3,4,5}, and
recently an analysis of boosted bound state equation for the $ep$ system was
presented in \cite{6}, while the $1+1 ~~e^+e^-$ case was considered in
\cite{7,8}.

Another approach (the $N$-quantum approach) was used in \cite{9}, while the WKB
method (expansion in powers of $\hbar$) in \cite{10}.

  A more convenient tool to study the effects of  boosting would be a
  Hamiltonian with e.g. instantaneous interaction, derived from the quantum
  field action. However this line of reasoning has  several complications.
  First of all, the  usual methods of introducing interaction via particle
  exchange - exclude the nonperturbative mechanisms, which produce confinement
  in QCD \cite{12}. Secondly, the Minkowskian particle  exchange automatically
  brings in the appearance  of  the  new Fock sectors  with  a new created
  particle in addition to the basic two-particle content. A way to handle this
  problem was suggested recently in \cite{7}. In a general case one obtains the
  matrix  Hamiltonian for the Fock column wavefunction, and one needs a
  systematic way to cut off the higher states to concentrate on the lowest
  ones.

  Moreover, one should have a simple way to disregard the spin degrees of
  freedom in the first approximation to make clear the dynamical mechanism of
  boosting.

  All these problems are economically treated in the path integral (world line)
  formalism \cite{13} based on the Fock-Feynman-Schwinger representation
  \cite{14}. Recently this formalism was presented in an especially useful form
  \cite{15}, where higher Fock state can be systematically eliminated, and the
  spin-dependent interaction treated separately \cite{16}. The accuracy of the
  first simple approximation in QCD and QED was checked in \cite{17}.

  As we show below, this formalism provides one with the Hamiltonian of an
  arbitrarily moving system with internal interaction, given by the Lorentz
  invariant construction -- the Wilson loop. The latter includes both
  nonperturbavive and perturbative  (particle exchange) interactions written
  first in the Euclidean space-time via field correlators and therefore does
  not produce higher Fock states, the latter appear due to perturbative quantum
  creation.

  Below we are using the path-integral formalism of \cite{15}, which provides
  the  Hamiltonian of a two-particle state in a moving coordinate system,
  where the total momentum $\veP$ of the state is  defined. Our formalism
  yields the Hamiltonian with  additional  parameters $\omega_1, \omega_2$,
  which play the role of  the  virtual particle energies, and the stationary
  point analysis of the state in terms of $\omega_1, \omega_2$,  exact  at
  large time interval of the system $T$, yields the energy $E$ of the moving
  state.

  It is  essential, that the interaction in the system is obtained in QCD and
  QED from  the Wilson loop, which is gauge and Lorentz invariant, and where
  the resulting instantaneous (or  light-cone) interaction is obtained via
  field correlators \cite{15}, see \cite{16*} for the corresponding light-cone
  work. In this way one can in principle define interaction in any moving
  system, however practically this task can be difficult. We are using general
  properties of the Wilson loop and make an ansatz for wave function. As  a
  result one can  find the approximate wave function and energy  of a given
  state in a moving coordinate system.

One should stress, that the study of the boosted dynamics by itself has not
much practical meaning, since all inertial systems are equivalent. However in
practice there are many processes, which include interactions of slow and  fast
particles, and, hence, possible overlap integrals of their wave  functions, and
here the knowledge of boosted dynamics is necessary, and as we show, it leads
to remarkable effects.

  In the present  paper we are addressing these problems for the QCD and QED
  bound states. We construct the Hamiltonian $H(\veP)$ of the two-body system
  and find its eigenvalues. We show that the eigenvalue in the moving system
  $E_0(\veP)$ can be found in the form
  \be E_0(\veP)= \sqrt{\veP^2 + \tilde M^2_0},\label{1m}\ee
  where $\tilde M_0$ is defined by the boosted interaction $V_{\veP}$ and
  should coincide with the c.m. energy $M_0$ provided $V_{\veP}$ is found
  correctly.

  Using the Wilson loop form, we find that the boost $L_{\veP}$ acts on the
  original c.m. interaction at least in two ways: reorganizing its magnitude
  $V\to CV$, and changing its coordinate dependence
  \be V_{\veP} = L_{\veP} V = CV (L \{\ver\})\label{2m}\ee

  From the general Lorentz invariance of the Wilson loop one finds that at the
  stationary points      \be C=C_0 = \sqrt{1-\left( \frac{v}{c}\right)^2 } =
  \frac{M_0}{E_0(\veP)}.\label{3m}\ee
  Note, that we shall put $c=1$ in what follows.
  Neglecting at first the second modification  $(V (\ver) \to V (L (\ver)))$,
  we check that the mass $\tilde M_0$ in (\ref{1m}) obtained in the moving
  system approximately coincides with the original mass eigenvalue calculated
  the c.m. system. We consider several examples of $V(\ver)$: 1) linear
  confinement, 2) gluon or photon exchange and in both cases we find that
  $\tilde M_0$ agrees with $M_0$ within 10\% or better.

  To check the full Lorentz covariance of our procedure with $\omega_1,
  \omega_2$ we consider the relativistic two-body system of noninteracting
  particles of different masses $m_1, m_2$ and apply our procedure.

  We find that indeed the eigenvalues $E_0(\vep)$ have the form (\ref{1m}), where $\tilde M_0$ is the c.m. of  two particles with the
  particle momenta $\vep_1=\vep, \vep_2=-\vep$ in the c.m. system, $\tilde M_0
  = M_0 (\vep, -\vep)$. Having checked this (global) invariance, one must
  consider the case  of the shape boosting  -- the so-called
  Lorentz--FitzGerald
  contraction \cite{17*}, which is the  result of the second    step in the
  boosting transformation $V(\ver) \to V (L (\ver)).$ This step cannot  be
  obtained directly and kinematically
  since the instantaneous interaction in one system is not Lorentz
  (kinematically) connected to the  instantaneous interaction in another
  moving system, and there occurs a serious  restructuring  of  the
  interaction.

  Therefore we impose the condition of the Lorentz contraction on the  wave function
  and interaction, and in this way we find the explicit form of $L(\ver)$ in
  (\ref{2m}). This condition, which plays the  role of an ansatz,  defines the
  wave function in any system, provided it is known in the c.m. frame. As a
  result one can connect the Lorentz  contracted wave function to the parton
  wave function at large $P$ and find,  that it has usual scaling properties,
  but interconnected transverse  and longitudinal dynamics. One also finds
  immediate consequences of Lorentz contraction for physical processes, e.g.
  for decay amplitudes, quark decay constants, form factors etc., part of which
  was discussed  before (see  e.g. \cite{2} and \cite{17**}), while other should be
  investigated in future.

  The paper is organized as follows. In the next section the general form of
  the path integral for two-body Green's function is written and the
  relativistic Hamiltonian is defined in terms of $\omega_1, \omega_2$ and
  Wilson loop interaction.

  In section 3 the case of the  two noninteracting particles is considered and
  the  general structure of Lorentz covariant eigenvalues $E_n=\sqrt{\veP^2 +
  M^2_n}$ is confirmed.

  In section 4 the global property of the boosted interaction $V\to CV, ~~ C=
  \frac{M_n}{E_n}$ is  derived from the Wilson loop  interaction and checked in
  the cases of Coulomb and confining interaction.

  The section 5 is devoted to the  Lorentz contraction ansatz and the ensuing
  properties of the wave function and interaction with possible consequences
  for physical effects. An appendix is devoted to the comparison of Lorentz
  contracted and scaled parton wave functions.

  In the last section the main results and approximations are reiterated and
  some prospectives are given.

\section{The QCD and QED path-integral Hamiltonian in  the moving  systems.}

The two-body $(q_1, \bar q_2)$ Green's function generated by the currents $j_i
= (\psi \Gamma_i \psi)$  in the relativistic path formalism \cite{15} can be
written in the Euclidean space-time \be G_{12} (x,y) = \frac{T}{2\pi}
\int^\infty_0 \frac{ d \omega_1}{\omega_1^{3/2}} \int^\infty_0
\frac{d\omega_2}{\omega_2^{3/2}} (D^3z^{(1)} D^3z^{(2)})_{\vex\vey}\lan \hat T
W_\sigma (A)\ran\label{2.1}\ee where $T$ is the Euclidean time interval, and
\be \lan \hat T W \ran = 4 tr Y \lan W \ran \exp (-K (\omega_1) - K(\omega_2)
), \label{2.2}\ee

\be Y= \frac14 \Gamma_1 (m_1 - i \hat p_1) \Gamma_2 (m_2 - i \hat
p_2)\label{m6}\ee and \be K(\omega) = \int^T_0 dt_E \left( \frac{\omega}{2} +
\frac{m^2}{2\omega} + \frac{\omega}{2} \left( \frac{ d\vez}{dt_E} \right)^2
\right), \label{2.3} \ee while $\lan W \ran $ is the Wilson loop, which can be
expressed via field correlators \be \lan W(C) \ran = \lan Tr \exp ig \int d
\pi_{\mu\nu} (z) F_{\mu\nu} (z) \ran= \exp \sum^\infty_{n=1} \frac{(ig)^n}{n!}
\int d\pi (1) ... d\pi(n) \llan F(1) ... F(n)\rran\label{2.4}\ee \be d\pi (i) =
d s_{\mu\nu} (z_{ i }) + i \sigma_{\mu\nu}
\frac{dt_i}{2\omega_i}.\label{2.5}\ee

As was shown in \cite{12} the leading quadratic in $F$ term in the cumulant
expansion (\ref{2.4}) in the c.m. frame yields  instantaneous confinement  and
gluon exchange interaction in the $3+1$ QCD case, and the Coulomb interaction
in $3+1$ QED

\be \lan W (C) \ran =\exp \left\{- \int V (r (t_E) ) dt_E+ {\rm spin~ dep.~
terms}\right\}\label{2.6}\ee \be V_{QCD} (r) = \sigma r -\frac43
\frac{\alpha_s}{r}, ~~ V_{QED} (r) =- \frac{\alpha}{r}.\label{2.7}\ee

It is clear that the vacuum averaging of $W(C)$, implied by the angular
brackets, yields higher order corrections to $\alpha_s,e^2$ and $ \sigma$.

We now turn to the case of the Hamiltonian in a moving Lorentz system. To this
end we define the $q_1\bar q_2$ Green's function and Hamiltonian in the system
with the total momentum $\veP$ \cite{15} $$G_P (x,y) = \frac{T}{2\pi}
\int^\infty_0 \frac{d\omega_1}{\omega_1^{3/2} }\int^\infty_0
\frac{d\omega_2}{\omega_2^{3/2}} Y d^3 (\vex-\vey)
e^{i\veP(\vex-\vey)}\times$$\be \times\lan \vex |e^{-H(\omega_1,\omega_2,
\vep_1, \vep_2)T}|\vey\ran\label{2.15}\ee with  \be H(\omega_1, \omega_2,
\vep_1,\vep_2) = \sum_i \frac{p^2_i + m^2_i + \omega^2_i}{2\omega_i} + \hat
V=\sum_{i=1,2} \frac{m^2_i + \omega^2_i}{2\omega_i} + \frac{\vepi^2}{2\tilde
\omega} + \frac{\veP^2}{2(\omega_1 + \omega_2)} + \hat V.\label{2.16}\ee Here
we have replaced the instantaneous c.m. coordinates $\vex_1$ and $\vex_2$, by
the relative and total c.m. coordinates \be \verho= \vex_1 -\vex_2, ~~\veR =
\frac{\omega_1 \vex_1 +\omega_2 \vex_2}{\omega_1+\omega_2},\label{2.17}\ee
$$\vepi = \frac{\partial}{i \partial \verho}, ~~\veP = \frac{\partial}{i\partial
\veR}.$$

Note, that $\vepi$ is not the c.m. momentum, the latter we denote for two
particles as $(\vep, -\vep)$.

 To have the lowest eigenvalue of $H(\omega_1,
\omega_2, \vep_1, \vep_2)$ one should calculate the minimal value of its
eigenvalue $E(\omega_1 , \omega_2, \veP)$ in the stationary value analysis with
respect to $\omega_1, \omega_2$ \be \left.\frac{\partial E (\omega_1, \omega_2
, \veP)}{\partial \omega_i}\right|_{\omega_i =\omega_i^{(0)}} = 0,~~ i=1,2; ~~
E_0 (\veP) \equiv E (\omega_1^{(0)} , \omega_2^{(0)}, \veP)\label{2.18}\ee

It is clear, that the instantaneous c.m. interaction $V_{cm}$ in (\ref{2.16})
will be changed by the Poincare boost  operator $\hat L(\veP)$ in the general
system, hence one can write for $\hat V$ in (\ref{2.16})\be\hat V = \hat L
(\veP) V_{cm}.\label{2.19}\ee

We expect that the eigenvalues of the operator (\ref{2.16}) after minimization
should have the form \be E_0 (\veP) = \sqrt{\veP^2 + M^2_0}\label{2.20}\ee
where $M_0$ is the c.m. energy of the $q_1\bar q_2$ system.

Note, that we have  neglected for simplicity spin-dependent forces originating
from $\sigma_{\mu\nu} \frac{dt}{2\omega}$ in (\ref{2.5}), see \cite{16} for
details and references. As a result our Hamiltonian is a $4\times 4$ unit
matrix in Dirac  indices. We shall check (\ref{2.20}) in the following chapters
in the examples of free particles and QCD and QED systems.

\section{The case of two noninteracting particles}

    In this case we define:
    \be \Omega\equiv \omega_1+\omega_2; ~~ \omega_1 =\Omega x, ~~\omega_2 =
    \Omega (1-x)\label{2.21}\ee
    \be H= \frac{\veP^2 +\Omega^2}{2\Omega}+ \frac{1}{2\Omega} M^2_0, ~~ M_0^2
    \equiv \frac{\vepi^2 + m^2_1}{x}+ \frac{\vepi^2+m^2_2}{1-x}.\label{2.22}\ee
    Minimizing $M_0^2$ in  the c.m. system, where $\vepi=\vep$ in the interval $x\in$[0,1] one obtains the stationary
    point $x_0 = \frac{\varepsilon_1}{\varepsilon_1+\varepsilon_2}$, where
    $\varepsilon_i = \sqrt{\vep^2+m^2_i}$, and  finally$M_0^2=
    (\varepsilon_1+\varepsilon_2)^2,$ so that minimizing finally in $\Omega$,
    one  has
    \be E_0 (\veP)=
    \sqrt{\veP^2+(\varepsilon_1+\varepsilon_2)^2}.\label{2.23}\ee

    Hence $\varepsilon_1 +\varepsilon_2$ is the c.m.energy of two free particles
    with masses $(m_1, m_2)$ and momenta $( \vep ,-\vep )$, and the Lorentz
    covariance of our expression is proved, if one assumes, that $M^2_0$ should  be  calculated in the c.m. system, where $\vepi =
    \vep$.Now one has to find the same  operator $M^2_0$ (\ref{2.22}) in the
    moving system.

We consider again  the Hamiltonian  for the free particle  motion, but now use
Lorentz transformations for momenta to  support the result  (\ref{2.23}) \be
H_0 = \frac{\veP^2}{2(\omega_1+\omega_2)} + \frac{\omega_1 + \omega_2}{2} +
\frac{\vepi^2}{2\tilde \omega} + \frac{m^2_1}{2\omega_1} +
\frac{m^2_2}{2\omega_2},\label{21m} \ee and all coordinates refer to the same
moment of time, $\tilde \omega =\frac{\omega_1\omega_2}{\omega_1+\omega_2}$.

In terms of individual momenta
 in the moving system  $\vep_i = \frac{1}{i} \frac{\partial}{\partial z_i}$,
 one can write
 \be \vep_1 = \frac{\omega_1}{\omega_1+\omega_2} \veP + \vepi, ~~ \vep_2 = \frac{\omega_2}{\omega_1+\omega_2} \veP -
 \vepi\label{22m}\ee
hence \be \veP = \vep_1 + \vep_2 , ~~ \vepi = \frac{\vep_1 \omega_2 - \vep_2
\omega_1}{\omega_1 + \omega_2}.\label{23m}\ee

Our next goal is to express $\vepi$ in terms of the relative c.m. momentum
$\vep  (c.m.) \equiv \vep$

Note, that the Hamiltonian (\ref{21m}) can be written as \be H_0 =
\frac{\vep^2_1+m^2_1 + \omega^2_1}{2\omega_1} + \frac{\vep^2_2 + m^2_2 +
\omega_2^2}{2\omega_2}\label{24v}\ee and the on-shell condition for $\omega_i$
is obtained from the stationary point analysis of (\ref{24v}) in terms of
$\omega_1$ and $\omega_2$. One has \be \omega_i^{(0)} = \sqrt{\vep^2_i +
m^2_i}, ~~ i=1,2.\label{25m}\ee

Hence $\omega_i^{(0)}$ plays the role of the particle energy and we shall below
always replace $\omega_i$ by  $\omega_i^{(0)}$, implying that both particles
are on the mass shell. We shall show that the eigenvalues of the   Hamiltonian
(\ref{21m}) satisfy Eq. (\ref{1m}) and $\tilde M_0$ is exactly equal to the
c.m. energy of two particles.

Introducing the velocity $v$ of the c.m. system, one can write \be \omega_1
=\frac{\bar \omega_1 + \vev\vep}{\sqrt{1-v^2}}, ~~ \omega_2 = \frac{\bar
\omega_2 - \vev\vep}{\sqrt{1-v^2}},\label{26m}\ee where  $\bar \omega_1$ are
particle energies in  the c.m. system. For parallel and perpendicular
components of $\vep_i$ w.r.t. $\vev$ in terms of the c.m. momenta $p_\|$ ,
$\vep_\bot$ one has \be p_1 (\|) = \frac{p_\|+v\bar\omega_1}{\sqrt{1-v^2}}, ~~
p_2 (\|) = \frac{-p_\|+v\bar\omega_2}{\sqrt{1-v^2}},\label{27m}\ee \be
p_1(\bot) = p_\bot, ~~ p_2 (\bot) = - p_\bot.\label{28m}\ee From (\ref{23m})
one obtains \be \vepi_\bot = \vep_\bot, ~~ \pi_\| = \frac{p_\|}{\sqrt{1-v^2}} +
\frac{v}{\sqrt{1-v^2}} \left( \frac{\omega_2 \bar \omega_1 - \omega_1 \bar
\omega_2}{\omega_1 + \omega_2}\right).\label{29m}\ee

Inserting (\ref{26m}) in  (\ref{29m}), one obtains \be \pi_\| = p_\|
\sqrt{1-v^2}\label{30m}\ee also $\omega_1  +\omega_2 = \frac{\bar \omega_1
+\bar \omega_2}{\sqrt{1-v^2}}$.

As a result $H_0$ assumes the form \be H_0 = \frac{\veP^2 \sqrt{1-v^2}}{2(\bar
\omega_1+ \bar \omega_2)} + \frac{\bar \omega_1 + \bar \omega_2}{2
\sqrt{1-v^2}} + \frac{\sqrt{1-v^2}}{2}\left \{ \frac{p^2_\| (1-v^2) + p^2_\bot
+ m^2_1}{\bar \omega_1 + \vev\vep} +\frac{p^2_\| (1-v^2) + p^2_\bot +
m^2_2}{\bar \omega_2 - \vev\vep} \right\}.\label{31m}\ee

Using $\bar \omega_i^2 = p^2_\| + p^2_\bot + m^2_i , ~~ i=1,2$ one finally
obtains \be H_0 = \frac{ \veP^2 \sqrt{1-v^2}}{2 (\bar \omega_1 + \bar
\omega_2)} + \frac{\bar \omega_1 + \bar \omega_2}{2 \sqrt{1- v^2}} + \frac{\bar
\omega_1 + \bar \omega_2}{2} \sqrt{1-v^2}.\label{32m}\ee One can express $v$ as
follows, $M_0 \equiv \bar \omega_1+\bar \omega_2$, \be v= \frac{P}{\sqrt{P^2
+M^2_0}}, ~~ \sqrt{1-v^2} = \frac{M_0}{\sqrt{P^2+M^2_0}}\label{33m}\ee and as a
result one has \be H_0 = \sqrt{\veP^2 + M^2_0} \label{33m*}\ee implying the
Lorentz covariance of our approach.

It is now easy to compare our results for the free relativistic particles with
that of the Newton-Wigner approach \cite{18}. there the c.m. relative momentum
$\vep$ and the total momentum $\veP$, defined as above in (\ref{22m}),
(\ref{23m}), are connected with the momentum $\vepi=\frac{1}{i}
\frac{\partial}{\partial\verho}$ as follows: \be \vep = \vepi + \frac{ (\vepi
\veP) \veP}{E_0 (\sqrt{\veP^2 + E^2_0 }+ E_0 )}.\label{34m}\ee

Here $\vep$ and $\veP$ are canonically conjugated to the relative and c.m.
coordinates  $\vex$ and $\veX$, defined as follows: \be \vex=\verho+ \frac{
(\verho \veP)\veP}{E_0 (\sqrt{\veP^2 + E^2_0 }+ E_0)} + \frac{ (\verho \veP)
\vep}{E_0 \bar \omega_1 \bar \omega_2} \left( \bar \omega_1 - \bar \omega_2 -
\frac{\vep \veP}{\sqrt{\veP^2 + E^2_0}}\right),\label{35m}\ee \be X_i = R_i -
\frac{S_{ik} P_k}{E_0 (\sqrt{\veP^2 + E^2_0 } + E_0)}\label{36m}\ee where \be
S_{ik} = \rho_i \pi_k - \rho_k \pi_i.\label{37}\ee One can use (\ref{33m}) to
reduce (\ref{34m}) to the simple result \be p_\| =\pi_\|
\frac{1}{\sqrt{1-v^2}}, ~~ p_\bot = \pi_\bot, \label{38m}\ee which coincides
with (\ref{29m}), (\ref{30m}). One can in principle express the total
Hamiltonian in terms of canonically conjugated coordinates $\vex, \veX$ and
momenta $\vep, \veP$ and proceed to solve with the interaction  taken into
account, which is a difficult road. Instead we shall investigate a simpler,
however approximate way,   where the boosted interaction is easier to
implement.

\section{Boosting QCD and QED interaction}

We return to the general form (\ref{2.16}) and discuss  the Lorentz boost of
the interaction. Note, that our result (\ref{2.16}) is obtained in the moving
Lorentz system. In particular, one can check, that $\int_C A_\mu dz_\mu$ as
well as $\int_S d s_{\mu\nu} F_{\mu\nu}$ is not only gauge, but also Lorentz
invariant structures.

Rewriting (\ref{2.6}) as \be \lan W\ran = \exp ( - i\bar V (\ver) T_M)
\label{39m}\ee one  can exploit the Einsteinian time  dilatation to predict,
that any averaged interaction obtained from the Wilson loop average, transforms
under Lorentz transformation  from system $K'$ to system $K {''}$, moving with
respect  to $K'$ with velocity $ v$ as follows \be\bar V' T' =  \bar V'' T'',
~~ T'' = \frac{T'}{\sqrt{1-v^2}}, ~~  V'' = \bar V'\sqrt{1-v^2}.\label{40m}\ee

This gives us the factor $C_0= \sqrt{1-v^2}$ announced in (\ref{3m}). However
in the off-shell form of the Hamiltonian (\ref{2.16}), before the stationary
analysis in $\Omega$ is done, we shall use the off shell form for  $C,
C=\frac{M_0}{\Omega}$, which reduces to $C_0$ at the stationary point
$\Omega=E_0$. Note, that  this is not the only effect of the system motion, and
we shall discuss the effect of the Lorentz contraction in section 5.

Let us now use the property (\ref{40m}) to calculate the mass $M^2_0$ for
different interactions. We shall write the Hamiltonian (\ref{2.16}) as \be H =
\frac{\veP^2}{2\Omega} + \frac{\Omega}{2} + \frac{\hat M^2_0}{2\Omega} , ~~
\frac{\hat M^2_0}{2\Omega} = \frac{\vepi^2}{2\tilde \omega} + C V (\vex) +
\frac{m_1}{2\omega_1}+ \frac{m^2_2}{2\omega_2}.\label{41m}\ee

We consider the cases of the Coulomb and linear interactions.

\begin{description}

    \item[1)]{\bf  The case of opposite charges in $\mathbf{3+1}$ QED}

    We now study eigenvalues of (\ref{2.16}), where $\hat V(\veP)$ is given by
    (\ref{2.19}) and we assume for simplicity, that $\hat L (\veP)$ may be
    represented by a simple factor, $\hat L(\veP)\to C (\veP)$.

    The eigenvalues of the equation
    \be\left(\frac{\vepi^2}{2\tilde \omega}- \frac{\alpha C}{r}\right)
    \varphi_n =\varepsilon_n\varphi_n\label{2.24}\ee are given by
    $\varepsilon_n =- \frac{\tilde \omega (\alpha C)^2}{2n^2}$ and the total
    energy is (notations are as in (\ref{2.21})),
    \be E(\omega_1, \omega_2, \veP) = \frac{\veP^2+\Omega^2}{2\Omega}+
    \sum_{i=1,2} \frac{m^2_i}{2\omega_i} - \frac{\tilde \omega
    (\alpha C)^2}{2n^2}.\label{2.25}\ee
    Writing $E(\omega_1,\omega_2,\veP)= E(\Omega, x,\veP)$, one obtains from
    the minimization in $x$,
    \be -\frac{m^2_1}{x^2} + \frac{m^2_2}{(1-x)^2} - \frac{(\Omega \alpha
    C)^2}{n^2} (1-2x) =0 .\label{2.26}\ee

For $m_1=m_2$ one obtains $x_0 =1/2, ~~ \omega_1^{(0)} = \omega_2^{(0)}\equiv
\omega_0$ \be E\left(\Omega, \frac12, \veP\right)=
\frac{\veP^2+\Omega^2}{2\Omega} + \frac{2m^2}{\Omega} - \frac{\Omega(\alpha
C)^2}{8n^2} \equiv \frac{\veP^2 +\Omega^2 +\mathcal{
M}^2_0}{2\Omega}.\label{2.26a}\ee Putting $C = \frac{\bar M}{\Omega}$, one
finds the minimum  of (\ref{2.26a}) varying in $\Omega$, which yields \be E_0
(\veP) = \sqrt{\veP^2+\mathcal{M}^2_0}, ~~ \Omega_0 =
\sqrt{P^2+\mathcal{M}_0^2},\label{2.27}\ee \be \mathcal{M}_0^2 =4m^2-
\frac{\alpha^2\bar M^2}{4n^2}.\label{2.28}\ee   Inserting $\bar
M=\mathcal{M}_0$ in (\ref{2.28}) one obtains \be \mathcal{M}_0 =
\frac{2m}{\sqrt{1+\frac{\alpha^2}{4n^2}}}.\label{2.29}\ee This is exactly the
spectrum found for the relativistic two-body Coulomb problem  neglecting spin
dependent and annihilation terms \cite{17}.

    \item[2)]{\bf The case of the linear confining potential in $\mathbf{3+1}$ QCD.}

    We are writing the Hamiltonian (\ref{2.16})  in the form

    \be H=\frac{\veP^2}{2\Omega} +\frac{\Omega}{2} + \frac{1}{2\Omega} \left(
    \frac{m_1^2}{x} + \frac{m^2_2}{1-x}+ \frac{\vepi^2}{x(1-x)} + 2
    \bar M  V(\ver)\right)\equiv \frac{\veP^2+\mathcal{M}^2_0}{2\Omega} +
    \frac{\Omega}{2}\label{2.30}\ee
    where we have denoted
    \be L(\veP)V_{cm} (\ver) =C V_{cm}
   (\ver),  ~~ C= \frac{\bar M}{\Omega},\label{2.31}\ee
and $\bar M$ can in principle depend on $\veP$ and $\vepi$, but we start with a
simple ansatz with $\bar M = const$.

For $m_1=m_2$ the minimization in $x$ yields $x_0 =\frac12 $ and \be
\mathcal{M}^2_0 = 4m^2 + \bar \varepsilon^2, ~~\varepsilon^2\varphi= (4\vepi^2
+ 2 \bar M  V(\ver))\varphi.\label{2.32}\ee For $V(\ver)=\sigma r$ the
eigenvalues of (\ref{2.32}) are known \cite{19}. \be \bar \varepsilon^2 =
(4\bar M\sigma)^{2/3} a_n, ~~ a_0 = 2.338, ~~ \mathcal{M}_0 = \sqrt{ 4m^2 + (4
\bar M \sigma)^{2/3} a_n}.\label{2.33}\ee Eqs. (\ref{2.32}), (\ref{2.33}) yield
solution for $\mathcal{M}_0 $ in the boosted system.

Let us now consider the massless case $m_1=m_2=0$ in (\ref{2.30}) and take
$\bar M  = \mathcal{M}_0 (c.m.)$, which we shall calculate below separately.
One has from (\ref{2.32}), (\ref{2.33}) \be \mathcal{M}_0^2 = (4\mathcal{M}_0
(c.m.) \sigma)^{2/3} a_n,\label{2.37}\ee while $ \mathcal{M}_0 (c.m.)$ is found
from (\ref{2.30})  with $\veP=0$ and $\bar M=\Omega$ \be H(c.m) =
\frac{\Omega}{2}+\frac{2\vepi^2}{\Omega}+\sigma r \to \mathcal{M}_0(c.m.) =
\frac{\Omega}{2} + \left( \frac{2}{\Omega}\right)^{1/3}\sigma^{2/3}
a_n.\label{2.38}\ee

Minimizing $\mathcal{M}_0 (c.m.)$ in $\Omega$ one obtains the standard
expression, commonly used in hadron spectra  \cite{19} \be \mathcal{M}_0 (c.m.)
= 4 \sqrt{\sigma} \left( \frac{a_n}{3}\right)^{3/4}.\label{2.39}\ee Insertion
of (\ref{2.39}) in (\ref{2.37}) immediately yields \be \mathcal{M}_0 = 3^{1/2}
(16)^{1/3} \sqrt{\sigma} \left( \frac{a_n}{3}\right)^{3/4} \approx 4.33
\sqrt{\sigma}  \left( \frac{a_n}{3}\right)^{3/4}.\label{2.40}\ee One can see,
that (\ref{2.39}) and (\ref{2.40}) coincide within the accuracy of 8\%, hence
one can use approximately the following boosting factor of the linear potential
\be L(\veP) V_{c.m.} (r) = \frac{\mathcal{M}_0 (c.m.)}{\Omega(\veP)} V_{c.m.}
(r).\label{2.41}\ee

\end{description}

\section{Lorentz contraction and the boosted shape of a  bound state in QCD and
QED}

The full (infinite) set of all paths for the two-body Green's function
(\ref{2.1}) can be studied by making intersection with the 3d hyperplane at
some fixed time $t_0$. In this way one obtains the density of the  state, given
by the wave function $\Psi_n$\be \rho_n (\vex, t) =\frac{1}{2 i} \left(\psi
\frac{\partial}{\partial t} \psi^+ - \psi^+\frac{\partial}{\partial t}
\psi\right) = E_n|\Psi_n (\vex, t)|^2.\label{57}\ee

For a boosted coordinate system  one can define the longitudinal and
perpendicular sizes of the system  $l_\|$ and $l_\bot$ \be l_\|= \int |x_\||
\rho_n (\vex, t) dV\label{58}\ee \be l_\bot= \int |\vex_\bot |\rho_n (\vex, t)
dV.\label{59}\ee

Since densities obey the invariance law \cite{17*}
 under Lorentz
transformations \be \rho (\vex, t ) d V = inv\label{60}\ee and $x_\|$ is
Lorentz contracted in a moving system, one expects the following  dependence of
$l_\|, l_\bot$ \be l_\| (v) = \sqrt{1-v^2} l_\| (0), ~~ l_\bot (v) = l_\bot
(0).\label{61}\ee

The  basic question is how   (\ref{61}) is maintained and supported by the
dynamics of the given system, i.e. what is the transformation law $L\{\ver\}$
in \be LV(\ver) = CV(L \{\ver\}).\label{62}\ee Instead of solving this point
for $V(\ver)$, we turn to the wave function  $\Psi_n (\vex, t)= e^{-i E_nt}
\varphi_n (\ver)$ and try to ensure the property (\ref{61}).

One  possible solution for $\varphi_n (\ver)$ to satisfy (\ref{58}), (\ref{59})
is \be L_P\varphi_n (r) =\varphi_n \left(x_\bot,
\frac{x_\|}{\sqrt{1-v^2}}\right)\label{63}\ee

On the other hand \be dV_v = (dx_\| d^2x_\bot )_v = \sqrt{1-v^2} (dx_\| d^2
x_\bot)_0\label{64}\ee so that Eq.(\ref{60}) is satisfied. Hence $$(l_\|)_v =
\int |x_\||E_n| \varphi_n \left( x_\bot, \frac{x_\|}{\sqrt{1-v^2}}\right) |^2
(dx_\| d^2 x_\bot)_v= $$\be= \sqrt{1-v^2} \int \tilde x_\|| M_0 |\varphi_n (
x_\bot, \tilde x_\|) |^2 d\tilde x_\| d^2 x_\bot = \sqrt{ 1- v^2}
(l_\|)_0,\label{65}\ee

where  we have used $\tilde x_\|= \frac{x_\|}{\sqrt{1-v^2}}=x_\|^{(0)}$, i.e.
the c.m. parallel coordinate.  The next question is what  kind of  dynamics can
ensure the transformation (\ref{63}).

We now turn to our Hamiltonian \be H=\frac{\veP^2}{2\Omega} +\frac{\Omega}{2} +
\frac{(h_0)_v}{2\Omega},\label{66}\ee where \be (h_0)_v = (4 \vepi^2_v+4 m^2 +
2 \bar M V_v), ~~V_v = LV_v, ~~\vepi^2_v = L \vepi^2\label{67}\ee

Note, that $\vepi$ is not canonical momentum and  in general the transformation
from the c.m. system with the instantaneous c.m. Hamiltonian $(h_0)_{cm}$ to
another instantaneous system with the total momentum $\veP$ is not provided by
Lorentz transformation. Therefore we start as before in section with the
assumption that $(h_0)_v$ should be first solved in the c.m. system, and this
result $(h_0)_{cm} \varphi_{cm} = M^2_0 \varphi_{cm}$ should be inserted as an
eigenvalue for $(h_0)_v$, i.e. $(h_0)_v \to (h_0)_{cm} = M^2_0$.

This assumption was proved to be true for the noninteracting pair in section 3
and approximately correct (within 10\%) for the typical interactions in section
4. We now generalize this assumption to specify  $\vepi^2_v$ and $V_v$, and to
this end we define \be (h_0)_v \varphi_v = M^2_0 \varphi_v , ~~ \varphi_v =
\varphi (x_\|^v, x_\bot^v)\label{68}\ee where \be x^v_\| =
\frac{x_\|}{\sqrt{1-v^2}}, ~~ x_\bot^v = x_\bot;~~ \pi^v_\|=\frac{1}{i}
\frac{\partial}{\partial x^v_\|},\label{69}\ee

\be \pi_\bot^2 = \frac{1}{i} \frac{\partial}{\partial x_\bot^v}, ~~ V_v =
V(x^v_\|, x^v_\bot).\label{70}\ee

As a result the equation $( h_0)_v \varphi_v = m_0^2\varphi_v$ reduces to the
c.m. equation $h_0 \varphi = M^2_0 \varphi$ by a simple change of variable
$x_\|$ with the same eigenvalue $M_0^2$. We now can write the boost
transformations for  $V$ and $\varphi_n$ as follows$$ V(r) =L V(X) \to CV
\left(x_\bot, \frac{x_\|}{\sqrt{1-v^2}}\right), ~~ C= \frac{M_0}{\Omega}
\to\sqrt{1-v^2},$$\be \varphi_n (x) \to \varphi_n^{(v)} (x) = \varphi_n \left(
x_\bot, \frac{x_\|}{\sqrt{1-v^2}}\right)\label{71}\ee with  the normalization
\be \int E_n |\varphi_n^{(v)} (x)|^2 d V_v =1= \int M_0^{(n)} | \varphi_n^{(0)}
(x) |^2 dV_0.\label{72}\ee

As a result the shape of the object will be transformed according to the
Lorentz contraction rule \be l_\| (v) = l_\bot (v) \sqrt{1-v^2}.\label{73}\ee

One of the immediate consequences of the form (\ref{72}) is the high momentum
asymptotics of the wave function \be \tilde \varphi_n^{(v)}(q) = \int
\varphi_n^{(v)} (\ver) e^{i\veq \ver} d^3 \ver = C_0 \tilde \varphi_0
(\veq_\bot, q_\| \sqrt{1-v^2}),\label{74}\ee where $\tilde
\varphi_0(q_\bot,q_\|)$ is the Fourier transformed c.m. wave function. One can
see in (\ref{74}), that in the case, when one of the constituents gets a large
momentum $\veQ(Q_\|,0,0)$, the boosted wave function has a  saturating limit up
to the factor $C_0$ namely
$$ \tilde \varphi_n^{(v)} (\veq + \veQ)= C_0 \tilde \varphi \left(\veq_\bot,
(q_\|+Q_\|) \sqrt{1-v^2_q}~\right)=$$\be
\begin{array}{c}{\longrightarrow}\\{{Q\to\infty}}\end{array} \frac{M_0}{Q} \tilde \varphi
\left(\veq_\bot, Q \frac{M_0}{\sqrt{Q^2+M^2_0}}\right) \to \frac{M_0}{Q} \tilde
\varphi (\veq_\bot, M_0)\label{75}\ee

As a second example we consider  the process of the strong  decay of a meson
$M_1$ in the state $n$ into a pair of hadrons $M_2, M_3$, which can be both
mesons or both baryons $B_2, B_3$. The corresponding amplitude can be written
for  the $B\bar B$ decay as \cite{20} $ ((\vep', \vep'')$ are two relative
momenta in the $3q$ system)\be J_{nB\bar B} (\vep) = \int y^{B\bar B}_{red}
\frac{d^3\vep'}{(2\pi)^3} \frac{d^3\vep''}{(2\pi)^3} \Psi^+_{n} (\vep-\vep'
-\vep'') \Psi_B (\vep', \vep'') \Psi_{\bar B} (-\vep', -\vep'')\label{76}\ee
and for the $M_2 M_3$ decay as \cite{21,22}.

\be J_{nn_2n_3} (\vep) = \int y^{M\bar M}_{red} \frac{d^3\veq}{(2\pi)^3}
\Psi^+_n (\vep + \veq) \Psi_{n_2} (\veq) \Psi_{n_3} ( \veq),\label{77}\ee where
$y_{red}$ contains the explicit decay parameters, which belong to the system at
rest of the initial meson, see \cite{20,21,22} for details.

It is important, that the boosted wave functions in both cases belong to the
decay products, moving with momenta $(\veP, - \veP)$, (where $M_1 = \sqrt{
M^2_2 + \veP^2} + \sqrt{M^2_3 + \veP^2},$) which grows as $M_1$, when $M_1$
lends to infinity.

As we have found in (\ref{74}), the momentum dependent wave function acquires
the factor $C_i= \sqrt{1-v^2_i}$ for each momentum, so that in (\ref{77})
$\psi_{n_i} (\veq) = C_i \varphi_{n_i} (\veq_\bot, q_\| \sqrt{1- v^2_i}),
i=2,3$ while in (\ref{76}) $$\Psi_B (\vep', \vep'') = (1- v^2_B) \varphi_B
(\vep_\bot', \vep_\bot'', p_\|'\sqrt{1-v^2_B}, p_\|''\sqrt{1-v^2_B})$$.

\begin{figure}[!htb]
\begin{center}
\includegraphics[angle=0,width=9 cm]{figbbar.eps}
\caption{The amplitude of the process $e^+e^- \to B\bar B$ with an intermediate
state $Q\bar Q(Q=u,d,s,...)$. The step $X$ in the process is a nonperturbative
double pair creation during a small time interval $\Delta t\sim \lambda\sim
0.1$ fm. }
\end{center}
\end{figure}

As a result $J_n$ behaves as \be J_{nB\bar B} \sim (1- v^2_B)^2\sim \left(
\frac{M^2_B}{M^2_B+\veP^2}\right)^2\label{78}\ee

 \be J_{nn_3n_3} \sim \sqrt{(1-v^2_2)
(1-v^2_3)} \sim \left(
\frac{M^2_2}{M^2_2+\vep^2}\frac{M^2_3}{M^2_3+\veP^2}\right)^{1/2}.\label{79}\ee

We can now turn to the processes $e^+e^-\to M_2 M_3$, $e^+e^- \to B\bar B$ and
the corresponding time-like formfactors, see Fig.1, and \cite{20} for details.

To this end we define the cross section \be \sigma (e^+e^- \to h \bar h) =
\frac{ 12 \pi \alpha^2 p}{E^3} \left| \sum_Q e_Q \sum_n \frac{\Psi_n (0)
\eta_{hQ} J_{nhh} (p)}{E_n - E + \frac{ i \Gamma_n}{2}} \right|^2,
\label{80}\ee where $h=M,B$ and $\eta_{hQ}$ is the spin-recoupling coefficient
and the time-like formfactor is proportional to (\ref{80}), $ F(Q_0) \sim
\frac{\sigma E^3}{p\alpha^24 \pi}$ where $Q_0 =E$

 Note, that the sum over $n$ with the energy
denominator has the same structure as in the total hadronic ratio $R$, and
brings in a constant up to possible logarithmic terms, see e.g.  \cite{24*} for
a discussion.

Therefore one obtains the following asymptotics of the formfactor, for mesons
and baryons  \be F_h (Q_0) \sim \left( \frac{M^2_h}{M^2_h + \vep^2}
\right)^{n_h}, ~~ h= M,B, n_M =1 , ~~ n_B=2.\label{81}\ee

Here $Q^2_0  = 4 (M^2_h + \vep^2)$. One can see, that the law (\ref{81})
coincides with the famous ``quark counting rule'' for  formfactors, found in
\cite{23}.

 Finally, one can connect our boosted wave function with the partonic function
 of the hadron, \cite{24}, which in the limit of high momentum $P$ can be
 written in the scaled form
 \be \Psi_N (\vep_1,...\vep_N)\to \psi (\{\vep_\bot^{(N)}\},
 x_1,...x_N)\label{79m}\ee
 where $x_i = \frac{p_\|^{(i)}}{P}$, and $\Psi$ is normalized in the Lorentz
 invariant way. We show below in the appendix, that for two  equal mass partons both
 functions are connected as (see Appendix for details)
 \be \psi_2 (\vep_\bot, x_1, x_2) = M_0 \sqrt{x_1x_2} (2\pi)^{-3/2} \tilde
 \varphi_0
 \left(p_\bot,  M_0\left( x_1 - \frac12\right)\right)\label{80m}\ee
 which implies, that $\tilde\varphi_0$ has a correct scaling limit and that transverse
 and longitudinal degrees of freedom are combined, e.g. for the $S$ wave one
 has $\tilde\varphi_0 = \varphi \left (\sqrt{ p^2_\bot + \left( x_1 - \frac12\right)^2 M^2_0}\right)$ and $M_0$ is the c.m.
 mass of the hadron.

 From(\ref{80m}) one can define the valence quark distribution function in the
 hadron  $D^q_h (x, k_\bot),$ e.g. for a meson
 \be D^q_h (x, k_\bot) = \frac{ E^2_h}{\varepsilon_1 \varepsilon_2} | \psi_2 (
 p_\bot, x) |^2 = \frac{M_0^2}{(2\pi)^3} \left|\tilde \varphi_0  \left(p_\bot,
 M_0\left(x-\frac12 \right)\right)\right|^2.\label{83}\ee

 Note, that (\ref{83}) does not show any singularities, as $\tilde\varphi_0$ is a
 monotonic Fourier transform of the static hadron wave function, and the
 corresponding quark distribution function $D^q_h (x) = \int d^2 k_\bot D^q_h
 (x, k_\bot)$ is decreasing for large $\left| x_1 - \frac12\right|$ and has a maximum at $x=\frac12$, and no peak around $x=0$.
  At this point one should remember,
 that we are treating the {\bf isolated} valence Fock component  without the multigluon Regge
 ladder Fock components, which bring in the expected singularity
  of $D^q_h(x)$ at $x$ small. Nevertheless $\tilde \varphi_0 (k_\bot, k_\|)$ can be a good
 starting approximation for the perturbative process evolution.

 One should stress again, that we have imposed the Lorentz contraction mechanism
 on the valence component only, while higher components ( wee partons) may
 create a more complicated picture.

 Therefore our valence component could be called the ``pure valence''
 component, which is different from the standard valence component , e.g. $u^v(x) =
 u(x) -\bar u(x)$, containing Regge ladder contribution,  and it has no singularities at small $x$.

 \section{Conclusion and prospectives}

 We have used path integral technic to calculate Hamiltonian and wave
 functions of the boosted system of two particles interacting via Wilson loop average. In  doing so we have neglected  all Fock
 components of the wave function except for the chosen $(q\bar q)$ or $(e_1
 e_2)$.

 This may be  called a quenched approximation, but inclusion of higher Fock
 components is technically possible, see  e.g. \cite{25}, \cite{26}. We have proceeded in
 in  the  following steps:

 1) We have used the Wilson loop interaction to prove, that  it  acquires due
 to the boost an overall reduction factor $C= \frac{M_0}{\Omega} \to \sqrt{1-v^2}$.

 2) We have  considered a free system of two relativistic particles with
 different masses $m_1, m_2$ and proved, that our Hamiltonian correctly
 describes  the spectrum  of the  boosted systems, when the relative motion
 part $(h_0)$ is computed in the c.m. system.

 3) Combining 1) and 2) we have  checked   that our boosted  Hamiltonian $H=
 \frac{\veP^2 + \Omega^2 + h_0}{2\Omega}, ~~ h_0 = h^{rel}_{kin} + 2 M_0 V$
 approximately (within 10\%) reproduces the  boosted spectrum
 $$ E(P) = \sqrt{\veP^2+ M^2_0}$$
 after the  minimization in $\Omega$ is imposed on $H$. This check was done for
 the Coulomb and confining interaction.

 4) We have used the Lorentz contraction phenomenon to formulate  the ``Lorentz
 contraction rule'', by which the two-body wave function in its
 dependence on the relative instantaneous coordinate $r$ in the moving system,
 behaves as $\varphi (\ver_\bot, \frac{r_\|}{\sqrt{1-v^2}})$, where $v$ is the
 velocity of the system.

 Correspondingly the Fourier transform of the wave function \\ $C\tilde \varphi
 (p_\bot, \sqrt{1-v^2} (p_\| +Q))$ appears to be sensitive to large momentum
 transfer $Q$,  only through the  factor $C_0=\sqrt{1-v^2}.$

 As a result we have shown, that the amplitude of the two-meson decay process
 with large decay energy is proportional to the product $[(1-v^2_1)
 (1-v^2_2)]^{1/2}$. Moreover, as a consequence, the time-like form factors of
 mesons and baryons behave as $\frac{1}{Q^2}$ and $\frac{1}{Q^4}$ respectively,
 i.e. the same way, as in the ``quark counting rule''.

 5) We have connected our Lorentz contracted wave function with the scaled
 partonic function and found a smooth limit between them. In this way one can
 insist, that our nonperturbative wave function can be used in hard processes,
 which opens a wide field  of applications. Note at this point, that the effect
 of Lorentz contracted wave functions was discussed before in the literature in
 different forms, see e.g. the first reference in \cite{2} for a discussion
 and additional references, and application to the reaction $\vep\bar{\vep} \to \pi\pi$
 in \cite{17**}. Within the framework of the ``Lorenz contraction rule'' the
 initial and  final wave functions entering in the hard   processes can be
 directly taken from the c.m. bound state wave function $\psi_{cm}$.  We also
 proved that the properly defined through $\psi_{cm}$   parton wave functions  have correct
 scaling limits not depending on the boost momentum $\veP$.

 The approach presented above,   calls for further study and applications in numerous
 processes, where boosted wave functions appear in initial and final states,
 e.g. in form factors, decay processes, etc.

 The author is grateful to B.L.Ioffe and O.V.Kancheli for useful discussions.
 This research was supported by the RFBR grant 1402-00395.

\vspace{2cm}
 \setcounter{equation}{0}
\renewcommand{\theequation}{A.\arabic{equation}}

\hfill {\it  Appendix  1}

\centerline{\it\large  Normalization of boosted many particle states}

 \vspace{1cm}

\setcounter{equation}{0} \def\theequation{A. \arabic{equation}}

We start with the normalization of the multiparton wave function \cite{24} \be
E(P) \int \prod^N_{i=1} \frac{d^3p_i}{\varepsilon_i} \delta \left(
P-\sum^n_{k=1} p_k\right)| \psi(p_1,... p_N)|^2 =1 , \varepsilon_i =
\sqrt{\vep^2_i + m^2_i}\label{A.1}\ee which in the limit of large $P$ for $x_k
= \frac{p_\|^{(k)}}{P}$ can be written as (fast moving partons) \be \int \prod
d^2 p_\bot^{(i)} \frac{dx_i}{x_i} \delta^{(2)} (\sum^N_{i=1} \vep_\bot^i)
\delta (1- \sum^N_{i=1} x_i) |\psi( p_\bot^{(i)} , x_i)|^2=1 .\label{A.2}\ee

For two partons our wave function (\ref{72}) is normalized as \be M_0 \int
|\tilde\varphi_0 (p_\bot, p_\|) | \frac{d^3p}{(2\pi)^3} =  E(P) ({1-v^2}) \int
|\tilde \varphi_0 (k_\bot, k_\| \sqrt{1-v^2}|^2 \frac{d^3k}{(2\pi)^3}
=1,\label{A.3}\ee and the parton wave function $\psi (p_1, p_2)$ in terms of
our $\varphi(k)$ is

\be \psi (p_1, p_2) = \sqrt{\frac{\varepsilon_1 \varepsilon_2
M_0^2}{E(P)(2\pi)^{3 }}  }  \tilde \varphi_0,  ~~ \sqrt{ 1-v^2} =
\frac{M_0}{\sqrt{P^2+M^2_0}}.\label{A.4}\ee

To express $k_\bot, k_\|$ via parton momenta $p_i$ one can use (\ref{27m});
hence \be p_\|^{(1)} = k_\|+ \frac{P}{M_0} \bar\omega_1= P x_1\label{a.5}\ee
where $M_0=\bar \omega_1 + \bar \omega_2$, (which is approximately true also
for interacting partons),  and for equal mass partons one has \be x_1 =
\frac{k_\|}{P} + \frac{\bar \omega_1}{M_0} \to \frac{k_\| \sqrt{1-v^2}}{M_0} +
\frac12.\label{a.6}\ee

 At large $P\gg M_0, $
  one has the scaling limit \be \psi(p_\bot^{(i)} , x_i) = \frac{M_0}{(2\pi)^{3/2}} \sqrt{x_1 x_2}
 \tilde \varphi_0 \left(p_\bot, x_1-\frac12\right).\label{A.5}\ee
In a similar way the multiparton wave function is connected to our wave
function $\varphi(\vepi_1,... \vepi_{N-1})$ as \be \psi_N (p_1, ... p_N) =
\frac{1}{ (2\pi)^{\frac32 (N-1)}} \prod^N_{i=1} \sqrt{M_0 x_i} \varphi_N
(p^{(i)}_\bot, M_0 (x_i- {\nu_i} )).\label{A.6}\ee One should  stress again,
that $\tilde \varphi_0$ has no on-shell singularities and there is no
factorization in $p_\bot^{(i)}, x_i,$ since at lowest angular momentum\\
$\tilde \varphi_0  \sim \tilde \varphi \left(  \sqrt{(p_\bot)^2 + M^2_0\left( x
- \frac12\right)^2}\right)$.

redpajama_set_name: RedPajamaArXiv


Feb 07, 2018 Compare And Contrast Essay Topics List In choosing the compare and contrast essay topics the writer ought to identify topics that they can explore comfortably.
Merely mentioning the similarities and differences is not enough if one cannot analyze the main ideas. Comic books versus novels; Offense versus May 13, 2012 Creating a solid thesis is a great start to getting on your way to understanding how to analyze two books in an essay and doing it successfully.
ComparisonContrast Essays Writing an Outline for an Essay Analyzing Two Novels Comparing themes and characters in novels are common.
you will be required to compare two novels. Comparing themes and characters in novels are common. How to Compare Two Novels in Comparative Essay. How to Teach Students to Organize and Write CompareContrast Essays. What's a Dystopian Novel, and Why Do Teens For a compare and contrast essay, you will need to find elements within the books that have some type of similarity, such as the characters or themes.
Oct 24, 2012 How To Write an Essay Comparing Two Books. Posted on October 24, The most important thing is the comparison. Each paragraph should have at least one quote from each book.
Introduction and Conclusion. The introduction doesnt have to be too impressive, just a few lines. Rephrase the question, name both of the book title A Comparison of Heart of Darkness and The Secret Agent This essay consists of two separate parts but the intention is that both these parts will prove to be relevant from the point of view of what this essay sets out to study. Looking for example or sample essay?
The following tips how to write a good college compare and contrast essay on two books will help you. Free tips on writing an essay comparing 2 books. 100 Best Traditional Compare and Contrast Essay Topics for Students Events (point to the differences and similarities of some historical events or episodes from the book) Situations (choose to compare two different cases or episodes from your life) two of them are similar to (comparison) andor different from (contrast) one another.
When writing such essays students make connections between texts or ideas, engage in critical thinking, and go Sample comparecontrast essay outline Here is a sample outline for an essay comparing and contrasting Achilles and Odysseus attitudes toward war.
This example is excerpted from the Excellence in Literature Handbook for Writers, which contains much more information on this topic and many others.


text:
Luciana: Dida and Taffarel are big inspirations to me
Luciana saved three penalties to snatch Ferroviaria a Libertadores final place
She discusses the dramatic night and upcoming opponents America
Luciana recalls almost quitting football in 2015
Euclid of Alexandria wrote a book about mathematical exceptions. Luciana of Araraquara is penning its sequel.
Indeed, while arithmeticians say around 75 per cent of penalties are successfully converted, Luciana says, 'Not while I'm in town'. Deep into Thursday evening, for the umpteenth time in her career, the 33-year-old emerged as the shootout hero, keeping out three spot-kicks to snatch Ferroviaria a place in the Copa Libertadores final.
Luciana, Brazil's first-choice goalkeeper at the FIFA Women's World Cup™ Canada 2015, spoke to FIFA.com about the showdown with America on Sunday evening, her semi-final heroics, learning from Dida and Taffarel, the Ferroviaria fans and a special tattoo.
In sudden death, Rebeca Fernandez had a penalty to put Universidad in the final. What was going through your mind as she was walking up to take it?
I heard Luana screaming, 'It's not over, Ana Alice.' I looked over and Ana Alice was distraught. Luana was screaming, 'Don't cry, (raises voice further) this is not over.' I said to myself, 'I cannot let this happen.' Ana Alice has been tremendous for us in this Libertadores. Game after game. I couldn't let her be the villain, it would have been a great injustice. I was absolutely determined to save it. I prayed to God, waited till the last moment so that I could go the right way, and thank God I managed to save it.
Did Ana Alice thank you after the game?
She came to me saying thanks, but I told her, 'It's me who has to thank you. You never let the ball get near my goal.' When it does, I have to do my best just like Ana Alice, the defenders and the rest of the team does all game.
How did you feel when you saved the last penalty to put Ferroviaria in the final?
Immense happiness. Such gratitude to God and my team-mates. We lost our first game 4-0. We were one penalty away from losing [in the semi-final]. All that goes through your head. What a moment.
Have you seen the reaction of your coach Lindsay Camila when you saved that penalty?
(Laughs) I saw, I saw! Down on her knees, crying. I thought it was really cool. Football is so emotional. We received a lot of criticism at the start of the campaign, so it was a moment of great relief, happiness. It's really emotional watching her get emotional!
Is your penalty-saving expertise a natural gift or something you have worked on?
Penalties are so decisive in football. How often do they determine championships? So I have practised facing penalties a lot, and I have also studied some of the great penalty-savers a lot – not just female ones but male too. Dida has always been someone I've admired a lot. Dida was always so emotionless, you never saw any expression in his face. I think I managed to get some of that from him. It's a big advantage because you need to be emotionless when you are a goalkeeper and even more so when you are facing penalties. I'm also a big fan of Taffarel. I'm old (laughs), so I was fortunate to see a lot of Dida and a bit of Taffarel. I've studied videos of Taffarel too. Dida and Taffarel are big inspirations to me. I really like and have tried to learn from Alisson, Weverton and Tadeu too. I believe the more you study and practice, the better you become.
You mentioned losing your opener 4-0, and you were on the cusp of going out after drawing your second outing. Can you believe you're reached the final?
We didn't expect to be thrashed in the first game. But it happens in football. You can let it drag you down, or you can be united and say, 'Let's go out there and put it right'. We had a chat in the dressing room after the game and it made us stronger. Nobody else believed in us, but we believed in ourselves. The draw wasn't the result we were looking for either, but we were calm, confident going into the third game, and we played really well and got the big victory we needed.
Corinthians, the overwhelming favourites to win the Libertadores, lost on penalties in the semi-finals. Did you feel a sense of relief that you wouldn't have to face such a strong team?
No, we wanted Corinthians in the final, we wanted another Brazilian team in the final. I have some good friends at Corinthians, and I was really sad they didn't reach the final. The same goes for Kindermann – we always want the Brazilian teams to do well. Corinthians are a magnificent team – there's no words to describe them. I hope they can put it behind them and win the third-place playoff. I know they'll be really cheering for us in the final. It doesn't matter if it's us, Corinthians, Kindermann. What matters is that we win this trophy for Brazil.
What do you think of America?
A really tough side. They're such warriors – they never give up until the very end. They have a lot of quality and we know they have so much fight in them, so we will have to match this. But we're very confident we will emerge victorious.
Can you tell us about the affection the Ferroviaria supporters have for you?
It's really moving. Ever since I first arrived in Araraquara in 2013, they have been so nice to me. When I was down and needed it, they showed me affection. The Ferroviaria supporters are really special. 'Love' – that's the only word I can use to describe the relationship between us. It feels really great to make them happy, and I really hope we can win this title for these incredible supporters.
One of them, Rafael Zocco, has a huge tattoo of you on his leg…
(Laughs) It's amazing. They told me about it and I didn't believe it. So they sent me a WhatsApp photo and I still thought it was fake, a photoshop. I didn't think any more of it but they me to see it in person and I couldn't believe my eyes! I never, ever imagined a fan would get a tattoo of me, yet alone one so big. I was really emotional when I saw it. What an honour!
All this may not have happened had you quit football in 2015…
I was really sad, really down. I'd had a tough time. I'd had enough of football. I wanted to walk away, but my family wouldn't let me. They supported me so much and, thank God, I returned to training and am here today, very happy to be doing what I love. I hope I am evening happier after the final!
FIFA.com newsAsamoah: Football is a sport that really brings people together
Rivers United completely embarrassed, Lobi 'Shipped' four goals in, in Rivers huge defeat
Rivers United completely embarrassed, Lobi 'Shipped' four goals in, in Rivers huge defeat
Prayer not working for MFM FC, as they were defeat at home by Akwa United
FIFA.com newsWatch the Football Law Annual Review live
Tokyo 2020 Olympic draws to be held at the Home of FIFA


Konexx USB Phone 2 PC is the ultimate low cost on-demand or voice activated recording solution.
Record telephone conversations digitally to your desktop PC or notebook PC. File the recordings for later retrieval and playback. Playback all of your important conversations, easily access and replay important details that transpired. Send personalized voice messages via e-mail to your clients for marketing campaigns. E-mail important dictation from your home to your office. Share necessary information with your colleagues by e-mailing the conversations as an attachment.
There is no room for error in business today. That is why you need to record and access to information that is accurate and easy to locate.
With the Konexx USB Phone 2 PC solution, you can easily turn your PC into an ultimate low-cost, high-quality digital recording solution that allow you to record telephone conversation, conference calls via a speakerphone, dictations of meetings via a microphone, Now you can record telephone conversations, meetings or dictation digitally to your PC or notebook. File the recordings for later retrieval and playback, e-mailed, or archived for future reference.
Ultimate low cost solution to record telephone conversation digitally to your PC.
Move it from one PC to another without needing to re-register the software for use on another computer. Use it in the office or while you are on the road with your laptop PC.
Have the ability to play computer audio files to a called party through the telephone set.
Have the ability to dictate recorded messages using an external microphone.
Ability to record meetings, calls made using the telephone sets, speakerphone, or an audio conference telephone.
Use it on laptop PC without having to connect to an AC power outlet.
Ability to insert "Beep Tone" generation to comply with the "two party notification" recording laws in some states.
With the USB Phone 2 PC solution, you can record telephone conversation, conference calls via a speakerphone, dictations or meetings. The USB Phone 2 PC comes with hardware to connect to your telephone handset or headset port for recording phone conversations. An optional connection for the supplied external microphone is provided for recording calls made on the speakerphone, meetings or dictation.
The USB Phone 2 PC enables the playback of audio files through the telephone set for parties at the other end of your call to hear them. User's of the USB Phone 2 PC can also enable a recording "Beep Tone" generation to comply with the "two party notification" recording laws in some states.
The USB Phone 2 PC records conversations directly to your computer. Recordings can be saved directly to your hard drive or a server. The recordings are stored in the form of a "wav" file. 1 hour of recording consumes only 5.6 MB of disk space. Recordings can be archived to a CD or DVD. Over 100 hours of recordings can be archived to a CD.
Save recorded telephone conversations as .WAV files! The Phone 2 PC Basic utilizes Konexx's patented Phone 2 PC Interface and recording software to translate your voice calls into compressed files that can be e-mailed, or archived for future reference. Features include playback, fast-forward, rewind, e-mail, and automatic file naming. Supplied with an external microphone for recording dictation, meetings or interviews.
Call Centre Edition Call Center Edition is designed for use in a location where management does not want the user to have any control over the recording process or have access to any of the feature settings, such as a call center agent's desk. Call Center Edition contains all the following capabilities found on the Advanced Edition.
Basic with Transcription The ultimate low cost on demand recording and transcription solution. Combine the power of the USB Phone 2 PC Basic with an easy to install, easy to use 3 Key Foot Pedal. The foot pedal allows the control of play, pause, rewind and fast forward functions facilitating transcribing of the recorded conversations.
Ideal for Healthcare, Insurance, Private Investigation or Financial institutions. Healthcare providers can save conversations with health care reimbursement providers directly to the PC or Network hard drive. Have a physical record that can be played back or emailed, for conflict resolution. A best practice method for eliminating he said she said and most importantly a great tool for assisting in timely payment collections.


Vintage Werkes Garage is a car, motorcycle and bicycle restoration shop in Athens, Georgia. At the Vintage Werkes we pride ourselves on resurrecting forgotten items and getting them back out in the world to be enjoyed. Here you will find some of our own projects and finds.
Found here on The Samba is a very well sorted 1976 914 2.o liter. The Porsche lineup for our Bicentennial included an impressive 5 models of sports cars. The 924, 928, 911, 912 and 914 were all available at your local Porsche+Audi dealership at some point in the year. This 914 is the last of the bread and a mid-engined Porsche didn't see light again until the Boxster in the late 90's. This particular 914 has had a full engine rebuild within the last three years and is very well sorted. Buy this now at $12k before they creep up with the rest of the 70's Porsches.


text:
Q: NSDate timeIntervalSinceNow and local timezone? I'm doing a calculation to find the NSTimeInterval between a known futureDate (which is in GMT/UTC) and the current time (and timezone) where the device currently resides.
NSTimeInterval approachInterval = [futureDate timeIntervalSinceNow];

I know that NSDate does not store any timeZone specific data, this rather being something that is calculated when the date needs displaying on the device.
My question is that from my initial tests (I'm currently in GMT+0001) it seems that the NSTimeInterval returned does not account for my local timezone. Do I have to manually calculate the timezone offset and remove that from my interval, and what would be the best way of doing that given that I can't supply an NSDate with a correct timezone (using timeIntervalSinceDate: for example)

A: NSDate represents a single point in time. It does not have (and does not need!!) a time zone. So "a known futureDate (which is in GMT/UTC)" or "I can't supply an NSDate with a correct timezone" does not make sense.
[futureDate timeIntervalSinceNow] returns the time interval between futureDate and the
current date and time and is completely independent of any time zones.
If you do not get the expected result, then perhaps your calculation of futureDate was wrong.