What to study Student Lifestyle Should international students take the ACT?
Just as with American students, there's no clear-cut yes-or-no answer. If you're applying to college in the United States, you will almost certainly have to take one of the big two college admissions tests, the SAT or the ACT (American College Testing). Most schools in the United States accept both exams, so this probably won't be a deciding factor.
However, there are definitely some important things to take into consideration, including your natural talents, your education, and the resources available in your country.
The ACT has both an English and a Reading test, equivalent to the SAT Verbal sections (but the ACT calls them "tests," rather than "sections"). For many international students, this is a determining factor in choosing which test to take: the overall, "composite" ACT score averages your scores from English, Reading, Math, and Science, while the SAT combines your scores by adding your Quantitative and Verbal sections. So in both cases, your mastery of English will affect about half of your score, not taking into account nuances of word problems on the math sections.
Some key differences: there's greater time pressure on the ACT, so if you find it difficult to work quickly in a foreign language, the ACT may not be for you. On the other hand, anecdotal evidence suggests that the SAT's reading comprehension and grammar questions are more nuanced. When choosing between the ACT and the SAT, you'll need to decide: do I want to approach questions faster or try more difficult questions? Reading passages on the ACT is also a little longer, generally, but vary less in complexity than SAT passages.
The best way to decide if you should take the ACT? Take an ACT practice test and see how you do compared to an SAT practice test.
In some countries, students' education becomes specialised very early on. By the time you're in high school, you may already have chosen a particular "path," even if this is as generalised as "science" or "humanities." If you are specialising in science, you may want to consider taking the ACT, although be careful: the test is made to test scientific reasoning far more than scientific facts, so practice first!
Because of this focus on reasoning, it's also important that you don't let yourself be scared off if you haven't taken a science course in a few years. Yes, you'll have a little catching up to do, but the scientific knowledge on the ACT is relatively basic. Check out an ACT study guide to see the exact concepts that the exam tests and how, and you'll see: thinking logically is more important than memorising the periodic table of elements on the ACT!
It's true that, unlike many American students, you may not have access to resources such as the PreACT, or a version of the ACT given to younger students. Furthermore, you'll be more limited by the ACT test dates available in your region (but note that SAT test dates are also more limited abroad). However, those are the two big limitations, and they apply just as much to the SAT as to the ACT.
Even just a few years ago, international students were put at a disadvantage when taking American college admissions tests because good prep options weren't available abroad: a lot of American students took classes or studied with books that could only be found in the U.S. However, today, tutors and classes are available around the world, and great Internet resources – many of them free – exist to help students from every country do the best that they can on the ACT and SAT, giving them a leg up in the admissions process.
At the end of the day, consider your options carefully when deciding whether to take the ACT or the SAT. You probably will have to take one or the other, though! Admissions offices appreciate seeing IB results, as well as those from similar tests, but usually still require a standardised American admissions test, as well as an English test (TOEFL or IELTS are the most popular).
Take your English test before your ACT or SAT so that you can sharpen your English skills well in advance of the exam.
That way, you can focus on mastering the test format so you can show off your skills to their best advantage when test day finally rolls around.
Special thanks to Rachel Kapelke-Dale for providing us with this article. Rachel is a test prep expert at Magoosh. She has a Bachelor of Arts from Brown University, an MA from the Université de Paris VII, and a PhD from University College London. She has taught test preparation and consulted on admissions practices for over eight years.


text:
\section{Introduction}
The renormalization of the  meson spectral function in nuclear
matter (for some early references, see
\cite{Hatsuda1,Bernard1,Bernard2,Brown,Hatsuda2,Ko} and a recent
review is~\cite{Saito})
attracted substantial interest in connection with  the
measurements of the di-lepton invariant mass spectra from heavy ion
collisions~\cite{Agakishev1,Masera,Agakishev2}.
Recently  experimental results on
$\omega$ and $\phi$ meson modification at normal nuclear densities
have been reported in experiments involving photon and proton
beams \cite{Ozawa,Trnka,Naruki,Muto,Tabaru,Lolos}. The most remarkable
result obtained in all these experiments is the anomalous $A$-dependence
of the $\phi$-meson production from nuclear targets. At the same time
the $A$-dependence of the $\omega$-meson production both in $\gamma{A}$ and
$p{A}$ interactions can be well understood.

At the threshold of elementary $\phi$-meson production, its
momentum in the laboratory system, {\it i.e.} with respect to nuclear
matter, is quite high and a substantial fraction of the $\phi$-mesons decay
outside the nucleus. Only that small fraction which decays inside the
nucleus would indicate a probable pole shift of the spectral function.
Therefore one could not
expect to  observe  a significant in-medium modification of the
$\phi$-meson  mass by measuring the di-leptonic or $K^+K^-$ invariant mass
spectra. However, it is very plausible to study the modification of the
$\phi$-meson width, since at low densities it is related to the imaginary
part of the forward $\phi{N}$ scattering
amplitude~\cite{Lenz,Dover,Friman1}. The latter determines the
$\phi$-meson distortion in the nucleus, which can be studied by
measuring the $A$-dependence of the $\phi$-meson production.

Such ideas motivated experiments on $\phi$-meson production from nuclei
at the KEK-PS~\cite{Tabaru}, SPRING-8 \cite{Ishikawa} and at
COSY \cite{Hartmann1}. Here we analyze recent results on incoherent
$\phi$-meson\,  photoproduction from \, nuclei \, collected at
SPRING-8~\cite{Ishikawa}, which indicate a substantial distortion of
the $\phi$-meson in finite nuclei. For consistency, we also
analyze data on coherent $\phi$-meson photoproduction collected at
Cornell some time ago \cite{McClellan1}. We investigate the role of single and
coupled  channel effects in $\phi$-meson photoproduction and provide
a possible explanation  of the observed anomaly.

The manuscript is organized as follows. In Sec.~2, we analyze the elementary
amplitudes $\gamma p \to \phi p$ and $\gamma p \to \omega p$ in terms of the
vector meson dominance model and compare to data taken at Cornell, ELSA and
SPRING-8. In Sec.~3, we study coherent and incoherent $\phi$-meson
photoproduction off nuclear targets in a single channel optical
model and show that such an
approach is not capable of describing the new data from SPRING-8. Coupled
channel scattering is considered in Sec.~4 and it is in particular shown that
the $A$-dependence of the SPRING-8 data can be understood in a two-step model,
including $\omega-\phi$ mixing and coupling to an intermediate pion. We also
add some speculations about the excitation of crypto-exotuic baryons with
hidden strangeness. Sec.~5 contains our conclusions.

\section{Vector Dominance Model}
\subsection{Data evaluation}
Considering quark-anti-quark fluctuations of the photon, the Vector
Dominance Model (VDM) assumes that intermediate hadronic $q{\bar q}$
states are entirely dominated by the neutral vector mesons. In that
sense the hadron-like photon~\cite{Stodolsky}
is a  superposition of all possible vector meson
states. The $\gamma{N}{\to}\phi{N}$ reaction can be decomposed into the
transition of the photon to a virtual vector meson $V$ followed by the
elastic or inelastic vector meson scattering on the target
nucleon. The invariant reaction amplitude follows as~\cite{Bauer,Paul}
\begin{eqnarray}
{\cal M}_{\gamma{N}{\to}\phi{N}} = \sum_{V}\frac{\sqrt{\pi\alpha}}{\gamma_V}
{\cal M}_{VN{\to}\phi N},
\label{ampli1}
\end{eqnarray}
where the summation is performed over vector meson states, $\alpha$ is
the fine structure constant, $\gamma_V$ is the photon coupling to
the vector meson $V$ and ${\cal M}_{VN{\to}\phi N}$ is the amplitude for the
$VN{\to}\phi{N}$ transition.

\begin{figure}[t]
\vspace*{-6mm}
\centerline{\hspace*{5mm}\psfig{file=spring2.ps,width=9.5cm,height=9.4cm}}
\vspace*{-2mm}
\caption{The forward $\gamma{p}{\to}\phi{p}$ differential cross
section as a function of photon energy. The data are taken from
Refs.\cite{Erbe,Ballam,Besch,Behrend,Barber,Atkinson,Busenitz,Derrick,Barth,Mibe}.
The lines show the calculations using Eq.(\ref{vdm1}) with $\alpha_\phi$=0
and for different values of $\sigma_{\phi{N}}$.}
\label{spring2}
\end{figure}

A direct determination of  $\gamma_V$ is possible through
vector meson decay into a lepton pair~\cite{Nambu}
\begin{eqnarray}
\Gamma(V{\to}l^+l^-)=\frac{\pi\alpha^2}{3\gamma_V^2}\sqrt{m_V^2-4m_l^2}
\left[1+\frac{2m_l^2}{m_V^2}\right],
\label{coupl1}
\end{eqnarray}
where $m_V$ and $m_l$ are the masses of vector meson and lepton, respectively.
Taking the di-electron decay width from Ref.~\cite{PDG}, the photon coupling to
the lightest vector mesons is given as
\begin{eqnarray}
\gamma_\rho{\div}\gamma_\omega{\div}\gamma_\phi =2.48{\div}8.53{\div}6.69.
\label{coupl2}
\end{eqnarray}
Although the couplings $\gamma_V$ can be determined
experimentally,  Eq.({\ref{ampli1}) does not indicate whether
non-diagonal, {\it i.e.} $\rho{N}{\to}\phi{N}$ and
$\omega{N}{\to}\phi{N}$, or diagonal $\phi{N}{\to}\phi{N}$ processes
dominate the $\phi$-meson photoproduction on the nucleon, since the
${\cal M}_{V\phi}$ amplitudes can not be measured. Furthermore, VDM
suggests that the virtual vector meson stemming from the photon becomes
real through the four-momentum $t$ transferred to the nucleon, which in
general requires the introduction of a form-factor in the interaction
vertices~\cite{Hufner,Sibirtsev1,Sibirtsev2}.

\begin{figure}[t]
\vspace*{-6mm}
\centerline{\hspace*{5mm}\psfig{file=spring2a.ps,width=9.5cm,height=9.4cm}}
\vspace*{-2mm}
\caption{Same as in Fig.\ref{spring2} for a low photon energy scale. The
solid circles show the results collected by SAPHIR~\cite{Barth}, while
the solid triangles are the measurements from SPRING-8~\cite{Mibe}.}
\label{spring2a}
\end{figure}

The next step in the VDM analysis is to consider only the diagonal
transition or elastic $V{N}{\to}V{N}$ scattering. The imaginary
part of the amplitude $f^\ast_{\phi{N}}(0)$ in the center of mass for
forward elastic  $\phi{N}{\to}\phi{N}$ scattering
is related to the $\phi{N}$ total cross section, $\sigma_{\phi{N}}$, by an
optical theorem as\footnote{It is clear that this formalism  holds for the
photoproduction of any vector meson $V{=}\rho$, $\omega$, $\phi$,
$J/\Psi,\ldots\,$.}
\begin{eqnarray}
\Im f^\ast_{\phi{N}{\to}\phi N}(q_\phi, \theta{=}0)=
\frac{q_\phi}{4\pi}\, \sigma_{\phi{N}},
\label{optic}
\end{eqnarray}
where $q_\phi$ and $\theta$ are the $\phi$-meson momentum
and scattering angle in the $\phi{N}$ center of mass system,
respectively. The amplitude $f^\ast_{\phi{N}}$ is related to the Lorentz
invariant scattering amplitude as
\begin{eqnarray}
{\cal M}_{\phi N{\to}\phi N}=-8\pi\,\, \sqrt{s}\,\,
f^\ast_{\phi{N}{\to}\phi N}(q_\phi, \theta),
\end{eqnarray}
with $s$ the invariant collision energy squared.
The $\gamma{N}{\to}\phi{N}$ differential cross section is
given in terms of the Lorentz invariant amplitude as
\begin{eqnarray}
\frac{d\sigma_{\gamma N{\to}\phi N}}{dt}=
\frac{|{\cal M}_{\gamma N{\to}\phi N}|^2}
{64\pi s q_\gamma^2},
\end{eqnarray}
where $q_\gamma$ is the photon momentum in the center of mass system. By
introducing the ratio of the real to the imaginary part of the forward
$\phi{N}$ scattering amplitude as $\alpha_\phi$, the
$\gamma{N}{\to}\phi{N}$ differential cross section at $t{=}0$ can be
written as\footnote{Note that the ${q^2_V}/{q^2_\gamma}$ ratio
was not included in most of the VDM analyses reviewed in
Ref.\cite{Bauer}. While this simplification might be applicable at high
energies, that is not the case for most of the data available
at $E_\gamma{<}10$~GeV, as is illustrated by Fig.\ref{spring2a}.}
\begin{eqnarray}
\left.{\frac{d\sigma_{\gamma N{\to}\phi N}}{dt}}\right|_{t{=}0}\!\!\!\!\!
=\frac{\alpha}{16\gamma_\phi^2} \, \frac{q^2_\phi}{q^2_\gamma}\,
(1+\alpha_\phi^2)\, \sigma_{\phi{N}}^2.
\label{vdm1}
\end{eqnarray}
Again, both the ratio $\alpha_\phi$ and the total $\phi{N}$ cross
section are unknown.
Thus VDM analysis of photoproduction data requires additional
assumptions.

It is believed that at high energies the hadronic forward scattering amplitudes
are purely imaginary. The data available \cite{PDG} for the $pp$, ${\bar p}p$,
$\pi^-p$, $\pi^+p$, $K^+p$ and $K^-p$ reactions indicate that the
ratios of the real
to imaginary parts of the forward scattering amplitudes are $\simeq$0.1
at $\sqrt{s}{>}$20~GeV. The $\alpha_\phi$ ratio was
measured~\cite{Alvensleben} through the interference between the
$\phi{\to}e^+e^-$ decay and the Bethe-Heitler production of
electron-positron pairs and it was found that
$\alpha_\phi{=}{-}0.48^{{+}0.33}_{{-}0.45}$ at photon energies
6${<}E_\gamma{<}$7.4~GeV. This result is too uncertain to be used
in the further analysis. To estimate the maximum value of
$\sigma_{\phi{N}}$, we apply $\alpha_\phi{=}0$. It is clear that any
non--vanishing ratio $\alpha_\phi$ would result in a reduction of the
$\phi{N}$ cross section that will be evaluated from the data in what follows.

Now Fig.~\ref{spring2} shows the available
data~\cite{Erbe,Ballam,Besch,Behrend,Barber,Atkinson,Busenitz,Derrick,Barth,Mibe}
on the forward $\gamma{p}{\to}\phi{p}$ differential cross section as a
function of the photon energy. The lines are the results using
Eq.~(\ref{vdm1}) obtained with $\alpha_\phi$=0 and for different values
of the total $\phi{N}$ cross section. Only one experimental point at
high energy~\cite{Derrick} needs a large  $\sigma_{\phi{N}}$, although
within experimental uncertainty this measurement is in agreement with
the data at photon energies below 10~GeV, which are also shown
in Fig.~\ref{spring2a}. Note that a large part of the data shown in
Fig.~\ref{spring2a} is in reasonable agreement with calculations done with
$\sigma_{\phi{N}}{\simeq}$11~mb.

\begin{figure}[t]
\vspace*{-7mm}
\centerline{\hspace*{5mm}\psfig{file=spring3.ps,width=9.5cm,height=9.4cm}}
\vspace*{-2mm}
\caption{The forward $\gamma{p}{\to}\omega{p}$ differential cross
section as a function of photon energy. The data are collected in
Ref.\cite{Sibirtsev1}.
The lines show the calculations based on Eq.~(\ref{vdm1})
with $\alpha_\omega$=0 and for different values of $\sigma_{\omega{N}}$.}
\label{spring3}
\end{figure}

Fig.~\ref{spring2a} demonstrates the
disagreement between the most recent measurements from SAPHIR~\cite{Barth}
and SPRING-8~\cite{Mibe}, which are shown by the solid circles and the solid
triangles, respectively. Note that both sets of data
contradict the VDM predictions. Although this discrepancy requires
special investigation we would like to make the following comments
relevant to the present study and VDM analysis of the data.

\subsection{Comments}
Let us discuss the observed discrepancy between the data and the VDM
description at low energies through inspection of
the forward $\gamma{p}{\to}\omega{p}$ differential cross section,
shown in Fig.~\ref{spring3} as a function of the photon
energy. The different symbols indicate the data collected in
Ref.\cite{Sibirtsev3}, while the solid lines show the VMD calculations
based on Eq.~(\ref{vdm1}) with the ratio $\alpha_\omega = 0$
and for different values of
$\sigma_{\omega{N}}$, respectively. The data at $E_\gamma{>}$10~GeV
are in good agreement with the VDM assuming that
20${<}\sigma_{\omega{N}}{<}$30~mb. The low energy $\gamma{p}{\to}\omega{p}$
data indicate an excess with respect to VDM that is well understood in
terms of the non-diagonal $\rho{N}{\to}\omega{N}$ transition given by
Eq.~(\ref{ampli1}). More precisely, this can be explained by a $\pi$-meson
exchange contribution~\cite{Bauer,Friman}. Indeed,  the dominant
$\omega$-meson decay mode is $\pi^+\pi^-\pi^0$, which in general
is described in terms ofthe transition $\omega{\to}\rho\pi$, followed by the
$\rho{\to}\pi\pi$ decay. Therefore it is natural to expect that the
non-diagonal $\rho{N}{\to}\omega{N}$ transition plays a substantial
role in (low-energy) $\omega$-meson photoproduction.

Most of the results on the forward photoproduction cross
section are determined through an extrapolation of the differential
$d\sigma{/}dt$ cross section over a certain range of $t$, not to
the maximal accesible value,
but rather to the point $t = 0$,  by applying a fit
of the form  $d\sigma{/}dt{=}A\exp(bt)$. This is the reason why the $t =0$
differential cross sections at low photon energies, shown in
Fig.~\ref{spring3},  do not vanish even though they are clearly
dominated by $\pi$-meson exchange. The extrapolation to different $t$
might explain the difference between the SAPHIR~\cite{Barth} and
SPRING-8~\cite{Mibe} the results and data available at higher energies.

Indeed, within the Born approximation the $\pi$-meson exchange contribution
vanishes~\cite{Sibirtsev3,Friman,Berman,Sibirtsev4}
at $t{=}0$. Here the minimal and maximal value of $t$ is given by
\begin{eqnarray}
t^\pm=m_V^2-\frac{s{-}m_N^2}{2s}\, \biggl(s+m_V^2-m_N^2
\nonumber \\ \mp\left[(s-m_V^2-m_N^2)^2
-4m_V^2m_N^2\right]^{1/2}\biggr)~,
\end{eqnarray}
with $m_V$ and $m_N$ the masses of the vector meson and nucleon,
respectively. At threshold, $\sqrt{s}{=}m_V{+}m_N$,
the four--momentum transfer squared is
\begin{eqnarray}
t^\pm=-\frac{m_N \, m_V^2}{m_N+m_V},
\end{eqnarray}
With increasing energy, $\sqrt{s}{\gg}m_V{+}m_N$,
\begin{eqnarray}
t^-\simeq m_V^2-\frac{(s-m_N^2)\,  m_V^2 }{s},
\end{eqnarray}
and $t^-$ approaches zero.

It is not obvious whether the extrapolation should be done to
$t{=}0$ or to $\theta{=}0$, as is explicitly shown by
Eq.~(\ref{optic}). Note that for elastic scattering $t^-{=}0$.
Actually the differential $\gamma{p}{\to}\phi{p}$
cross sections measured by SAPHIR~\cite{Barth} and SPRING-8~\cite{Mibe}
shown in Fig.\ref{spring2a} were extrapolated to $t{=}t^-$ and the
$t{=}0$ correction in that case is $\exp{(-t^-)}$,
which accounts for a factor of $\simeq 1.61$ at the $\phi$-meson
photoproduction threshold.

Keeping that in mind one might conclude
that similar to the $\gamma{p}{\to}\omega{p}$ data the forward
$\gamma{p}{\to}\phi{p}$ differential cross section indicates some
enhancement with respect to the diagonal VDM. This enhancement might
stem from non-diagonal
transitions\footnote{Both SAPHIR and SPRING-8 measurements of angular
spectra in the Gottfried-Jackson frame support this conclusion.}.
Apparently that problem requires additional investigation, which is
beyond the scope of the current study.

Moreover the discrepancy between the  SAPHIR~\cite{Barth} and
SPRING-8~\cite{Mibe} results can be partially explained by the
different range of $t$ used for the $t{=}t^-$ extrapolation.
SPRING-8 explored the range $t{-}t^-{>} 0.4~{\rm GeV}^2$, while the
SAPHIR measurements were used to fit $d\sigma{/}dt$ over a
larger range and at maximum photon energy $t{-}t^- > -2~{\rm GeV}^2$.
For that reason it is worthwhile to
reanalyze the SAPHIR data by fitting the differential cross section with
the sum of a soft and a hard component.

Finally,  keeping in mind the uncertainty of the analysis of  low
energy data on the forward $\gamma{p}{\to}\phi{p}$ differential cross
section we conclude that VDM yields the upper limit of the total
$\phi{p}$ cross section about 11~mb. If the ratio of the
real to imaginary forward scattering amplitude, {\it i.e.}
$\alpha_\phi$, is not equal to zero, then $\sigma_{\phi{p}}$ can be
even smaller, as  indicated by Eq.(\ref{vdm1}).

\section{Single channel optical model}
Consider a nuclear reaction as a succession of collisions of the
incident particle with individual nucleons of the target. If the
nucleus is sufficiently large the reaction can be formulated in terms
of  the optical model through replacement of the multiple individual
interactions by an effective potential interaction with nuclear matter.
Within the so-called $t\rho$ approximation that is valid at normal nuclear
densities, $\rho$=0.16~fm$^{-3}$, the optical potential is given by the
product of the density and forward two-body scattering amplitude. Similarly,
the Glauber theory expresses the cross section for reactions on nuclear
target in terms of elementary two body
interactions~\cite{Glauber,Yennie,Bochmann1}.

Conversely, by measuring
the nuclear cross sections it might be possible to study the
elementary interactions~\cite{Bauer}.  The realization of Drell and
Trefil~\cite{Drell} and Margolis~\cite{Margolis} that such a formalism
could be used to study the interaction of unstable
particles with the nucleon by producing them in a nucleus with hadronic or
electromagnetic beams, stimulated enormous experimental
activity~\cite{Bauer}. This method was first
applied~\cite{Drell,Margolis,Kolbig} for the evaluation of the $\rho{N}$
interaction from coherent and incoherent $\rho$-meson photoproduction
off nuclei. Coherent photoproduction has the advantage that the
produced particle must have quantum numbers similar to those of the
photon.

\subsection{Coherent photoproduction}
An extensive study of  coherent $\phi$-meson photoproduction
on a variety of nuclear targets was
done at the Cornell 10 GeV electron
synchrotron~\cite{McClellan1}. One might expect~\cite{Margolis,Kolbig} the
$A$--dependence of coherent photoproduction at high energies
to be proportional to $A^2$
if  the $\phi$-meson  does not interact in nuclei,
{\it i.e.} if it is not distorted by  final state interactions (FSI).
By fitting the forward $\phi$ meson photoproduction cross
section~\cite{McClellan1} with a function $\sim A^\alpha$, one obtains
the slope $\alpha{=}1.37{\pm}0.08$ at the photon energy of 6.4~GeV and
$\alpha{=}1.53{\pm}0.05$ at $E_\gamma = 8.3$~GeV.
The shaded boxes in Fig.~\ref{spring1b} show these results,
which indicate a strong deviation from a dependence on $A^2$.

Note, however, that the forward photoproduction cross
section contains both coherent and incoherent contributions. In
the absence of the FSI distortion, the incoherent photoproduction
cross section is proportional to $A$. Therefore one might argue that
the $A$-dependence  results from a
mixture of  coherent and incoherent $\phi$-meson photoproduction.
In order to verify such a possibility, an additional experiment with
linearly polarized photons with average energy of 5.7~GeV was
performed~\cite{McClellan2}. The measured polarization asymmetry
for the forward
$\phi$-meson photoproduction from a carbon target was found to be consistent
with the assumption of coherent photoproduction\footnote{At the same time the
asymmetry from the hydrogen target seems to be inconsistent with purely
elastic $\phi$-meson photoproduction. As we discussed in Sec.~2
this Cornell observation~\cite{McClellan2} is in agreement with the most
recent results from SAPHIR~\cite{Barth} and SPRING-8~\cite{Mibe}.}.

\begin{figure}[t]
\vspace*{-6mm}
\centerline{\hspace*{3mm}\psfig{file=spring1b.ps,width=9.5cm,height=9.4cm}}
\vspace*{-3mm}
\caption{The slope $\alpha$ of the
$A^\alpha$ dependence of the forward $\phi$-meson photoproduction
cross section as a function of the total $\phi{N}$ cross section. The
shaded boxes indicate the results
at photon energies 6.4 and 8.3 GeV obtained at
Cornell~\cite{McClellan1}.  The
lines show the calculations by Eq.(\ref{finalc}) with different
longitudinal momenta $q_l$=0 (solid), 63 (dashed) and 82~MeV/c
(dotted), which are fixed to the photon energy by Eq.(\ref{long}). The
calculations were done for the ratio $\alpha_\phi{=}0$.}
\label{spring1b}
\end{figure}

In order to evaluate the $\phi{N}$ interaction from coherent
photoproduction one can apply the method proposed in
Refs.~\cite{Margolis,Kolbig} and express the
amplitude for coherent $\phi$-meson photoproduction from nuclei
as~\cite{Bauer,Drell,Kolbig,Ross1,Trefil1,Trefil2}
\begin{eqnarray}
{\cal T}^{coh}_{\gamma{A}{\to}\phi A}(t,A)=
{\cal T}_{\gamma{N}{\to}\phi N}
\!\int\limits^\infty_0\!d^2b
\, J_0(q_t\,b)
\nonumber \\  \times
\!\!\int\limits^\infty_{-\infty}\!\!dz \,\rho(b,z)
  \exp{[iq_lz]}\times\left[1-i\chi_{\phi}(b,z)\right]^{A-1},
\label{ampl1}
\end{eqnarray}
where ${\cal T}_{\gamma{N}}$ is the elementary photoproduction amplitude
on a nucleon, an integration is performed over the impact parameter $b$, the
$z$ coordinate is along the beam direction and
$\rho(r{=}\sqrt{b^2{+}z^2})$
is the nuclear density function normalized to the number of the
nucleons in the nucleus.
Here, $t$ is the four-momentum transferred to the nucleus and
${-}t = q_l^2 + q_t^2$, with $q_l$ and  $q_t$ being  the
longitudinal and transverse component, respectively,
given by
\begin{equation}
q_l = k-\cos\theta\sqrt{k^2-m_\phi^2}, \hspace{5mm}
q_t = \sin{\theta}\sqrt{k^2-m_\phi^2},
\label{long}
\end{equation}
where $k$ is the photon momentum, $m_\phi$ is the
pole mass of the $\phi$-meson and $\theta$ is the emission angle of the
produced $\phi$-meson. In Eq.~(\ref{ampl1})
$J_0$ is the zero order Bessel function. The last term of
Eq.~(\ref{ampl1}) accounts for the distortion of the  $\phi$-meson
through an effective interaction with  $A{-}1$ nuclear nucleons and
$\chi_{\phi}$ is the corresponding nuclear phase shift.
Here we neglect the distortion of the photon.
The phase shift $\chi_{\phi}$ can be well approximated
within the impulse approximation by~\cite{Newton,Sibirtsev5}
\begin{equation}
\chi_{\phi}(b,z) =  -\frac{2\pi \, f_{\phi{N}}(p_\phi,\theta{=}0)}{p_\phi}
\int\limits^\infty_z\!\rho(b,y)\, dy,
\label{phase1}
\end{equation}
where $f_{\phi{N}}$ is the complex amplitude for the forward
$\phi{N}$ elastic scattering taken now in the rest--frame with respect to
the nucleus, {\it i.e.} in the laboratory system. Note that $p_\phi$ is
$\phi$-meson momentum in the laboratory frame.
The imaginary part of $f_{\phi{N}}$ amplitude is related
through the optical theorem to the total cross section
$\sigma_{\phi{N}}$ similar to Eq.(\ref{optic}), replacing $q_\phi$
by $p_\phi$.

By introducing the ratio of the real to imaginary part of the forward
$\phi{N}$ scattering amplitude, $\alpha_\phi$, the  cross section for
coherent $\phi$-meson photoproduction from nuclei is finally given as
\begin{eqnarray}
\frac{d\sigma_{\gamma A{\to}\phi A}^{coh}}{dt}=
\frac{d\sigma_{\gamma{N}{\to}\phi N}}{dt}
\left|\,
\int\limits^\infty_0\!d^2b\,\,
J_0(q_tb)\!\int\limits^\infty_{-\infty}\!\!dz \,\rho(b,z)
\right. \nonumber \\ \left.\times \exp{[iq_lz]} \,
\exp\left[\frac{\sigma_{\phi{N}}\, (i\alpha_\phi{-}1)}{2}
\int\limits^\infty_z\!\rho(b,y)\, dy\right]\right|^2\!\!\!\!.\,\,\,\,\,
\,\,\,\,\,
\label{finalc}
\end{eqnarray}
The general features of the coherent photoproduction are as
follows.  The $t$-dependence is given by the elementary
$\gamma{N}{\to}\phi{N}$ photoproduction amplitude as well as by the
nuclear form factor. The differential cross section has a diffractive
structure due to the $J_0(q_tb)$ dependence. However, up to now this
structure was not observed experimentally, since it is non--trivial to
isolate coherent from incoherent photoproduction, which dominates at
large $|t|$. The forward coherent $\gamma{A}{\to}\phi{A}$
photoproduction cross section
might be used for the extraction of the elementary forward
$\gamma{N}{\to}\phi{N}$ cross section, which can be compared with
those collected in Fig.\ref{spring2}. The $A$--dependence of
coherent photoproduction allows one to extract $\sigma_{\phi{N}}$ only
under certain constraints on $\alpha_\phi$. That extraction
is independent of the VDM assumptions.

\begin{figure}[t]
\vspace*{-8mm}
\centerline{\hspace*{3mm}\psfig{file=spring5b.ps,width=9.5cm,height=12.cm}}
\vspace*{-7mm}
\caption{The forward $\gamma{A}{\to}\phi{A}$ differential cross
section as a function of the mass number. The symbols show the data
collected at Cornell~\cite{McClellan1} at photon energies 6.4
(circles) and 8.3~GeV (squares). The lines are the calculations with
the total $\phi{N}$ cross section of 10 (solid), 30 (dashed) and 50~mb
(dotted) and with the ratio $\alpha_\phi{=}0$. Both experimental
results and calculations are divided by $A$. The calculations are
normalized at the $A{=}12$ point.}
\label{spring5b}
\end{figure}

Indeed if the distortion of the $\phi$-meson is negligible and
$q_l{=}0$ the coherent photoproduction cross section is proportional
to $A^2$ as is given by Eq.(\ref{finalc}). Furthermore, to analyze the Cornell
data and for completeness, we specified the density distribution
function $\rho(r)$ used in Eq.(\ref{finalc}) as
\begin{eqnarray}
\rho(r)=\frac{\rho_0}{1+\exp[(r-R)/d]},
\end{eqnarray}
with parameters
\begin{eqnarray}
R{=}1.28A^{1/3}{-}0.76{+}0.8A^{-1/3}\,\, {\rm fm},
\,\,\,\,\,\, d=\sqrt{3}/\pi \,\, {\rm fm},
\end{eqnarray}
for the nuclei with $A{>}16$. For light nuclei we
adopt~\cite{Dalkarov,Alkhasov}
\begin{eqnarray}
\rho(r)=(R\sqrt{\pi})^{-3}\left[4+\frac{2(A-4)r^2}{3R^2}
\right]\exp[-r^2/R^2],
\end{eqnarray}
with $R{=}\sqrt{2.5}$~fm.

We note that the results on forward photoproduction are not
sensitive to the variation of the ratio $\alpha_\phi$, as can be seen
from Eq.(\ref{finalc}) and is known from the analyses of $\rho$-meson
photoproduction~\cite{Bauer} and hadronic elastic
scattering~\cite{Sibirtsev5}.

Finally, the lines in Fig.~\ref{spring1b} are
the calculations based on Eq.~(\ref{finalc}) with momentum $q_l = 82$
(dashed) and 63 (dotted) and 0~MeV/c (solid),  related to the
photon energy by Eq.~(\ref{long}). The results are shown as a function
of the total $\phi{N}$ cross section. The calculations for  $q_l$=0~MeV/c
correspond to the high energy limit, {\it i.e.} $k{\gg}m_\phi$, and
for $\sigma_{\phi{N}}$=0 actually match the $A^2$
point. To get the slope $\alpha$ we fit our calculation with the function
$cA^\alpha$ with $c$ a constant and using the set of nuclear
targets corresponding to the experimentals.
Fig.~\ref{spring1b} illustrates that the $q_l$ correction
already introduces a substantial departure from the
$A^2$-dependence. Although the uncertainties in the  $\sigma_{\phi{N}}$
extraction from the data are large, the data are in very good
agreement with the calculations with a total $\phi{N}$ cross section
of $\simeq 10$~mb.

Fig.~\ref{spring5b} shows the forward $\gamma{A}{\to}\phi{A}$
differential cross section as a function of the target mass
number $A$. The circles and
squares are the experimental results obtained at Cornell for photon
energies of 6.4 and 8.3~GeV, respectively. The lines show the
calculations for different $\sigma_{\phi{N}}$ and for the ratio
$\alpha_\phi{=}0$. Both data and calculations are
divided\footnote{Although in view of Eq.(\ref{finalc}) it is more natural
to  divide the results on coherent photoproduction by $A^2$, it turns
out that $A^{-1}$ representation is more illustrative in case of the observed
moderate $A$-dependence of the data and therefore is
very frequently used.} by $A$. Obviously the shape of the
$A$-dependence is different for the calculation  for the various
$\sigma_{\phi{N}}$. The experimental results are in perfect agreement with
the calculations using $\sigma_{\phi{N}}{=}10$~mb.

Finally,  one can as well extract the
elementary $\gamma{N}{\to}\phi{N}$ forward differential cross section
using Eq.(\ref{finalc}) and compare the results with the results
obtained by direct measurement.
The calculations with $\sigma_{\phi{N}}$=10 mb can be well fitted to
the data with an elementary $\gamma{N}{\to}\phi{N}$ forward differential
cross section around $2.2{-}2.6$ $\mu$b/GeV$^2$, which is in good agreement
with the results collected in Fig.\ref{spring2}.

\subsection{Incoherent photoproduction}
Recently incoherent $\phi$-meson photoproduction at photon energies
1.5${\le}E_\gamma{\le}$2.4~GeV was studied by the SPRING-8
Collaboration~\cite{Ishikawa}. The data were published with arbitrary
normalization and provide the $A$ dependence fitted by the function
$A^\alpha$ with slope $\alpha{=}0.72{\pm}0.07$.

The optical model expression for the incoherent photoproduction
including only the excitation of the single nucleon and
neglecting the Pauli principle, which suppresses the cross section at small
$t$, is given by~\cite{Bauer}
\begin{eqnarray}
\frac{d\sigma_{\gamma A{\to}\phi A}^{inc}}{dt}{=}
\frac{d\sigma_{\gamma{N}{\to}\phi N}}{dt}\!\!
\int\limits^\infty_0\!\!d^2b\!\!
\!\int\limits^\infty_{-\infty}\!\!\!dz \,\rho(b,z) \nonumber \\
\exp\Bigl[{-}\sigma_{\phi{N}}\!\!\!\int\limits^\infty_z\!\!\!\rho(b,y)\,
dy\Bigr]~.
\label{inco1}
\end{eqnarray}
Now if $\sigma_{\phi{N}} = 0$, the forward cross section is
proportional to $A$. The
shaded box in Fig.~\ref{spring1} shows the result from SPRING-8, while
the line indicates the calculations based on Eq.~(\ref{inco1}) for different
values of the total $\phi{N}$ cross section. Again, we fit our results
by the function $cA^\alpha$ and use the set of nuclear targets from
experiment\footnote{The $A^\alpha$ function is not the  dependence
given by  Eq.~(\ref{inco1}) and  only provides a useful representation of
the data. Indeed the slope $\alpha$ depends on the set of target
numbers $A$ used in the calculations. Therefore it is necessary to
simulate the experimental conditions explicitely.}. It is clear that the
experimental results favor $ 23 \le \sigma_{\phi{N}} \le  63$~mb. This is in
agreement with the experimental finding~\cite{Ishikawa} given as
$\sigma_{\phi{N}}= 35^{+17}_{-11}$~mb. The Pauli blocking corrections
make almost no change to the $A$-dependence and only suppress the absolute
value of the forward photoproduction cross section~\cite{Bauer,Cabrera}.

\begin{figure}[t]
\vspace*{-6mm}
\centerline{\hspace*{3mm}\psfig{file=spring1.ps,width=9.5cm,height=9.4cm}}
\vspace*{-4mm}
\caption{The slope $\alpha$ of the
$A^\alpha$ dependence of the incoherent $\phi$-meson photoproduction
cross section as a function of the total $\phi{N}$ cross section. The
shaded boxes indicate the results
at photon energies 1.5${\le}E_\gamma{\le}$2.4~GeV obtained by
SPRING-8~\cite{Ishikawa}.  The
lines show the calculations by Eq.(\ref{inco1}).}
\label{spring1}
\end{figure}

Clearly this result  differs substantially from the total
$\phi{N}$ cross section extracted from coherent $\phi$-meson
photoproduction. There are no available explanations why the distortion
of the incoherently produced $\phi$-meson is so extremely strong.
Furthermore, the calculations~\cite{Cabrera,Munlich} wich include  the
in-medium  modification of the $\phi$-mesoncannot account for such strong
distortion.

\section{Coupled channel scattering}
Since $\phi$ and $\omega$ mesons have the same quantum numbers, these
two states should mix with each other - see e.g.~\cite{Ross2,Trefil3,Sandra}.
Therefore the $\phi$-meson might be produced indirectly,
{\it i.e.} through the photoproduction of the $\omega$-meson followed
by  the $\omega{\to}\phi$ transition. Furthermore, there can in
principle occur an arbitrary
number of  $\omega{\leftrightarrow}\phi$ transitions. Moreover,
these transitions can occur either due to the $\omega$ and $\phi$
mixing, {\it i.e.} similar to oscillations, or because of the
$\omega{N}{\to}\phi{N}$ interaction. This is illustrated in Fig.~\ref{fig:mix}.
Since both $\omega$ and $\phi$
mesons are strongly interacting particles, their final state interaction
in any nuclear target would cause distortions.

\begin{figure}[t]
\vspace*{2mm}
\centerline{\hspace*{3mm}\psfig{file=Amix.eps,width=6.3cm,height=5.cm}}
\caption{Mechanisms of $\omega \to \phi$ conversion: a) direct
$\omega-\phi$ mixing amplitude and b) the $\omega{N}{\to}\phi{N}$ interaction,
where $N$ denotes a nucleon. Type b)  contains the direct mechanism a) besides
other effects. }
\label{fig:mix}
\end{figure}

The coupled channel scattering
apparently depends on the strength of the
$\omega{\leftrightarrow}\phi$ transition. However, one
expects the $\phi$-meson distortion to be considerable because of
the interference effect. Even a small amount of an
$\omega{-}\phi$ admixture might have a considerable effect on
$\phi$-meson production from complex nuclei. First discussed by Ross
and Stodolsky~\cite{Ross1,Ross2}, this effect has subsequently been largely
overlooked in the literature~\cite{Bauer}. Here we consider coherent
and incoherent $\phi$-meson photoproduction from nuclei within the
coupled channel approach.

\subsection{Coherent photoproduction}
The generalization of the single channel amplitude of
for the two coupled channel scattering can be done
by introducing the 2$\times$2 matrix instead of the last term of
Eq.(\ref{ampl1}) as
\begin{eqnarray}
\left( \begin{array}{cc}
\!\!\!\!\!\!\!\!1{-}\displaystyle\frac{\sigma_{\omega{N}}}{2}
\int\limits^\infty_z\!\!\rho(b,y)\,dy
& \!\!\!\!\!\!\!\!\!\!\!\displaystyle\frac{{-}\Sigma_{\omega\phi}}{2}
\!\!\!
\int\limits^\infty_z\!\!
\exp[i{\tilde q}_ly]\rho(b,y)dy\\
 & \\
\displaystyle\frac{{-}\Sigma_{\omega\phi}}{2}\!\!\!
\int\limits^\infty_z\!\!
\exp[-i{\tilde q}_ly]\rho(b,y)dy & \!\!\!\!
1{-}\displaystyle\frac{\sigma_{\phi{N}}}{2}
\!\!\!
\int\limits^\infty_z\!\!\rho(b,y)\,dy
\end{array} \right)\,\,\,
\label{matrix}
\end{eqnarray}
where we have used Eqs.~(\ref{optic},\ref{phase1}) and we denote by $\Sigma$
the effective $\omega{\to}\phi$ and  $\phi{\to}\omega$ transition
cross section, which are equivalent because of time-reversal
invariance. Furthermore, we neglect the real parts of the elastic and
transition amplitudes, since even in the single channel analysis they
could not be fixed. Furthermore, the longitudinal momentum
${\tilde q}_l$ is defined as
\begin{eqnarray}
{\tilde q}_l \simeq \frac{m_\phi^2-m_\omega^2}{2k}~.
\end{eqnarray}
Neglecting the off-diagonal transition, {\it i.e.} setting $\Sigma = 0$,
the matrix of Eq.~(\ref{matrix}) allows one to recover the single channel
optical model for $\omega$ and $\phi$-meson photoproduction, while
taking the elementary ${\cal T}_{\gamma{N}}$ amplitude as a two-component
vector.

\begin{figure}[t]
\vspace*{-8mm}
\centerline{\hspace*{3mm}\psfig{file=spring5c.ps,width=9.5cm,height=12.cm}}
\vspace*{-7mm}
\caption{The forward $\gamma{A}{\to}\phi{A}$ differential cross
section as a function of the mass number. The symbols show the data
collected at Cornell~\cite{McClellan1} at photon energies 6.4
(circles) and 8.3~GeV (squares). The lines are the coupled channel scattering
calculations by Eq.(\ref{two}) with the total $\phi{N}$ cross section
of  11~mb and the $\omega{N}$ cross section of 23~mb and for the
transition $\Sigma$=0 (solid), 0.3 (dashed) and 0.5~mb (dotted).
 Both experimental results and calculations are divided by $A$. The
normalization of the calculations is fixed by VDM as explained in the
text.}
\label{spring5c}
\end{figure}

Since in our case  $\Sigma$ is small, the amplitude for
coherent $\phi$-meson photoproduction from a nucleus can be expressed in
a simple form,
\begin{eqnarray}
{\cal T}_{\gamma A{\to}\phi A}^{coh}{=}\int\limits^\infty_0\!\!
d^2b\,\,  J_0(q_tb) \!\!
\int\limits^\infty_{-\infty}\!\! dz \, \rho(b,z) \, \exp[iq_lz]
\nonumber \\ \times\left(  {\cal T}_{\gamma N{\to}\omega N}
\displaystyle\frac{-\Sigma \int\limits^\infty_z\,\,  \exp[i{\tilde q}_ly]\,\,
\rho(b,y)\, dy}{(\sigma_{\phi N}{-}\sigma_{\omega N})
\int\limits_z^\infty \rho(b,y)\, dy}  \right. \nonumber \\ \left.
 \times \left[\exp[-\frac{\sigma_{\omega N}}{2}\!\!\!\int\limits_z^\infty
\!\!\rho(b,y)\, dy]{-}
\exp[-\frac{\sigma_{\phi N}}{2}\!\!\!\int\limits_z^\infty
\!\!\rho(b,y)\,dy]\right] \nonumber \right. \\ \left.
+{\cal T}_{\gamma N{\to}\phi N}\exp[-\frac{\sigma_{\phi N}}{2}
\!\!\!\int\limits_z^\infty\!\!\rho(b,y)\,dy]\right).\,\,\,\,
\label{two}
\end{eqnarray}
For $\Sigma{=}0$, Eq.~(\ref{two}) reduces to Eq.~(\ref{ampl1}) and
the coherent differential cross section is given by
Eq.~(\ref{finalc}). Moreover, Eq.~(\ref{two}) corresponds to the first
order perturbation expansion in $\Sigma$, {\it i.e.} the inclusion of only
one $\omega{\to}\phi$ transition. If $\Sigma$ is large one should
consider an arbitrary number of  $\omega{\leftrightarrow}\phi$
transitions, which might be done through the series
expansion~\cite{Benhar} of the off--diagonal elements of the matrix given
by Eq.~(\ref{matrix}).

Moreover in high energy limit, {\it i.e.} when $q_l{=}{\tilde
q}_l = 0$, the integration along $z$ can be done analytically and the
coherent  photoproduction amplitude is then  given in a well-known
form~\cite{Kolbig}
\begin{eqnarray}
{\cal T}_{\gamma A{\to}\phi A}^{coh}{=}\int\limits^\infty_0\!\!
d^2b\,\,  J_0(q_tb) \left[ \frac{{\cal T}_{\gamma N{\to}\omega
N}\,\,\Sigma}
{\sigma_{\omega{N}}{-}\sigma_{\phi{N}}} \right. \,\,\,\,\nonumber \\
\times\left(\frac{1{-}\exp{[-\displaystyle\frac{\sigma_{\omega{N}} \, T(b) }{2}
]}}{\sigma_{\omega{N}}}
-\frac{1{-}\exp{[-\displaystyle\frac{\sigma_{\phi{N}} \, T(b)}{2}]}}
{\sigma_{\phi{N}}}\right) \nonumber
\\\left.+\frac{{\cal T}_{\gamma N{\to}\phi
N}}{\sigma_{\phi{N}}}
\left(1{-}\exp{[-\displaystyle\frac{\sigma_{\phi{N}} \, T(b)}{2}]}
\right)\right],\,\,\,\,\,\,
\label{limit}
\end{eqnarray}
where the real parts of the scattering amplitudes were neglected and
the  thickness function is given as
\begin{eqnarray}
T(b)=\!\!\int\limits_{-\infty}^\infty
\!\!\rho(b,z)\,dz.
\label{tb}
\end{eqnarray}

Following the VDM results shown in Figs.\ref{spring2},\ref{spring3} we
use the  elementary elastic $\omega$ and $\phi$-meson photoproduction
amplitude given by Eq.\ref{vdm1}, namely as
\begin{eqnarray}
{\cal T}_{\gamma
N{\to}VN}=\frac{\sqrt{\alpha}}{4\gamma_V}\frac{q_V}{q_\gamma}
\sigma_{VN},
\end{eqnarray}
with the $\gamma_\phi$ and $\gamma_\omega$ coupling constants given by
Eq.(\ref{coupl2}) and with
$\sigma_{\phi N}{=}11$~mb and $\sigma_{\omega N}$=23~mb. Thus the
absolute normalization of our calculations is fixed by VDM.
Fig.\ref{spring5c} shows the coherent  $\gamma{A}{\to}\phi{A}$
differential cross section as a function of the mass number calculated
for different values of $\Sigma$. The data~\cite{McClellan1} might be
well reproduced by calculations with
$0{\le}\Sigma{\le}0.3$~mb. Only the experimental results at
$E_\gamma{=}6.4$~GeV support the coupled channel effect originating
from the $\omega{\to}\phi$ transition.

\subsection{Incoherent photoproduction}
Let us now consider incoherent photoproduction of $\omega$-mesons followed by
$\omega{N}{\to}\phi{N}$ scattering. Note that in the coupled
channel description of
coherent $\phi$-meson photoproduction the $\omega{\to}\phi$
transition is not necessaryly due to  the scattering on the target nucleon, but
might be also an oscillation due to the mixing. In that sense
incoherent photoproduction is given as a two step process and
differential cross section can be written
as~\cite{Bochmann1,Faldt,Vercellin}
\begin{eqnarray}
\frac{d\sigma_{\gamma A{\to}\phi A}^{inc}}{dt}{=}
\frac{d\sigma_{\gamma{N}{\to}\omega N}}{dt}\!\!
\int\limits^\infty_0\!\!{\tilde \Sigma} \, d^2b
\left[\frac{1-\exp[-\sigma_{\phi N}\, T(b)]}{\sigma_{\phi N}}
\right. \nonumber \\
\left. -\frac{\exp[-\sigma_{\omega N}\, T(b)]{-}\exp[-\sigma_{\phi N}\,
T(b)]}
{\sigma_{\phi N}-\sigma_{\omega N}} \right],\,\,\,\,\,
\label{inco2}
\end{eqnarray}
where the function $T(b)$ is given by Eq.(\ref{tb}) and it is not necessary
that $\Sigma = {\tilde \Sigma}$. Considering both  direct
and two-step $\phi$-meson production, one should in principle
add the contribution  given by Eq.(\ref{inco1}).

Unfortunately the data~\cite{Ishikawa} on incoherent $\phi$-meson
photoproduction from nuclei are given with arbitrary normalization and
we cannot investigate how big the possible contribution from
two-step production might be, since ${\tilde\Sigma}$ is unknown. However, it is
possible to examine the $A$-dependence due to the two-step process.

\begin{figure}[t]
\vspace*{-6mm}
\centerline{\hspace*{3mm}\psfig{file=spring6.ps,width=9.5cm,height=9.4cm}}
\vspace*{-7mm}
\caption{The incoherent $\phi$-meson photoproduction  cross
section as a function of the mass number. The circles show the data
collected at SPRING-8~\cite{Ishikawa}. The solid line is the coupled
channel scattering calculations by Eq.(\ref{inco2}) with the total
$\phi{N}$ cross section of  11~mb and the $\omega{N}$ cross section of
23~mb, while the dashed line is result obtained with   $\sigma_{\phi
N}$=11~mb and  $\sigma_{\omega N}$=30~mb.
The dotted line is the single channel results for $\sigma_{\phi N}$=11~mb.
Both experimental results and calculations are divided by $A$. The
normalization of the calculations is fixed at the $Al$ target.}
\label{spring6}
\end{figure}

Fig.~\ref{spring6} shows the incoherent $\phi$-meson photoproduction
cross section as a function of the target mass
measured at SPRING-8~\cite{Ishikawa}. The dotted line shows the
calculations performed within the single channel optical model using
Eq.(\ref{inco1}) with $\sigma_{\phi N} = 11$~mb.
The solid line represents the result obtained with the
coupled channel model calculation, Eq.(\ref{inco2}),
using $\sigma_{\phi N} = 11$~mb and $\sigma_{\omega N} = 23$~mb.
Both the data and our results are divided by $A$. The calculations are
normalized for an $Al$ target. The single channel calculations are
identical to the ones shown in
Refs.~\cite{Ishikawa,Cabrera,Munlich} and apparently can not
reproduce the data, as we already discussed in Sec.3.2. The two-step
model calculations are in reasonable agreement with experimental
results - providing an $A$-dependence ${\propto}A^{0.63}$. Thus the
measured $A$-dependence clearly indicates the dominance of the two-step
process in $\phi$-meson photoproduction. Unfortunately there are no
data available for heavy targets, which clearly are crucial for the
verification of the calculated $A$-dependence shown in
Fig.~\ref{spring6}.

Note that another two-step process, {\it i.e.} $\gamma{N}{\to}\pi{N}$
followed by $\pi{N}{\to}\phi{N}$ transition, would produce almost the same
dependence, ${\propto}A^{0.63}$, as shown by the dashed line in
Fig.\ref{spring6}. In the considered $\pi$-meson momentum range the
total $\pi{N}$ cross section is about $\simeq$30~mb and therefore
calculations were done using Eq.(\ref{inco2}) with $\sigma_{\omega
N}$=30~mb. Note that both $\pi$-meson photoproduction and the
$\pi{N}{\to}\phi{N}$ transition are quite large and therefore
it is possible that  incoherent $\phi$-meson photoproduction is
dominated by a two--step reaction mechanism. For instance theoretical
studies~\cite{Cassing1,Sibirtsev6,Debowski,Sibirtsev7,Paryev} on low
energy $K^+$, $\rho$, $\omega$ and $\phi$-meson production in proton
nucleus collisions indicate dominance of the two-step process with
intermediate $\pi$-mesons. This result is strongly supported by
measurements of the $A$-dependence and two-particle correlations in
$K^+$-meson production from $pA$
reactions~\cite{Debowski,Koptev1,Badala,Buescher1,Koptev2}.
Further investigations on incoherent $\phi$-meson photoproduction
require measurement of  differential cross section with
absolute normalization.

It is also clear that incoherent coupled channel $\phi$-meson
photoproduction might also proceed through  coherent $\omega$
meson production by the photon, followed by the incoherent
$\omega{\to}\phi$ transition. This mechanism involves, in addition,
substantial $q_l$-dependence at low photon energies
similar to that of Eq.(\ref{finalc}), which allows
for  freedom in description of the $A$-dependence.

\subsection{Estimates for {\boldmath$\Sigma$} and
{\boldmath${\tilde\Sigma}$}}

It is useful to estimate the $\Sigma$ and ${\tilde\Sigma}$
in order to understand how large the effect due to the
$\omega{\to}\phi$ transition might be. Our
estimates are based on the amplitudes evaluated in free space, which
are not necessarily the same as in nuclear matter.

Very recently the the $\omega{-}\phi$ mixing amplitude
$\Theta_{\omega\phi}$  was investigated~\cite{Kucurkarslan} within
the leading order chiral perturbation theory and it was found that
$\Theta_{\omega\phi}{=}(25.34{\pm}2.39){\times}10^{-3}$~GeV$^2$. In our
normalization $\Sigma$ can be related to $\Theta_{\omega\phi}$
as~\cite{Urech}
\begin{eqnarray}
\Sigma \simeq \frac{1}{m_\omega^2}
\frac{\Theta_{\omega\phi}^2}{(m_\phi^2-m_\omega^2)^2} = 2.2
{\rm \mu b},
\end{eqnarray}
where we neglect the width of the $\omega$ and $\phi$-meson.
Actually the effect due to the $\omega{-}\phi$ mixing is small and as
is indicated by the calculations shown in Fig.\ref{spring5c} might be
supported by the Cornel data~\cite{McClellan1} on coherent
$\phi$-meson photoproduction from nuclei. However, the data itself do
not really require the inclusion of the mixing amplitude and the problem still
remains open.

The contribution to incoherent $\phi$-meson photoproduction from the
two step process with an intermediate
$\pi$-meson can be reasonably estimated since there are data available for
the $\pi{N}{\to}\phi{N}$ reaction collected in
Refs.\cite{Sibirtsev8,Sibirtsev9} and parameterized as
\begin{eqnarray}
{\tilde\Sigma}(\pi{N}{\to}\phi{N})=\frac{18\sqrt{s-s_0}}
{0.1285+(s-s_0)^2}\,\,\ {\rm \mu b},
\end{eqnarray}
where $s$ is the squared invariant mass of the $\pi{N}$ system given
in GeV$^2$ and
$\sqrt{s_0}{=}m_N{+}m_\phi$ is the reaction threshold. Note that at pion
energies of$\simeq 2$~GeV, which correspond to the forward $\phi$-meson
photoproduction in the SPRING-8 experiment~\cite{Ishikawa} the
$\pi{N}{\to}\phi{N}$ cross section is about 20~$\mu$b. Furthermore, at
photon energies of 1.5${\le}E_\gamma{\le}$2.4~GeV the total cross section
for the $\gamma{N}{\to}\phi{N}$ reaction is in average
$\simeq$0.3~$\mu$b~\cite{Sibirtsev10}
while the  $\gamma{N}{\to}\pi{N}$ reaction accounts for
$\simeq$5~$\mu$b~\cite{Kellett,Landolt}. Therefore the contribution
from the two-step mechanism might be well suppressed as compared to the
direct $\phi$-meson photoproduction. This can be clearly seen by
inspecting Eqs.(\ref{inco1},{\ref{inco2}) and replacing the $\omega{N}$
intermediate state with the $\pi{N}$ one.

It is difficult to estimate reliably the contribution to incoherent
$\phi$-meson photoproduction from a two-step process
with an intermediate $\omega$-meson. Figs.\ref{spring2a},\ref{spring3}
illustrate that incoherent forward
$\omega$-meson photoproduction dominates
$\phi$-meson photoproduction  by a factor of order$\simeq 60$.
However, at the same time the
$\gamma{p}{\to}\phi{p}$ data collected in Fig.\ref{spring3}
show almost no room for the non-diagonal $\omega{N}{\to}\phi{N}$
transition. The data at low photon energies are well described by the
VDM accounting only for elastic diagonal $\phi{N}{\to}\phi{N}$
scattering. Within the experimental uncertainties of the forward
$\gamma{p}{\to}\phi{p}$ differential cross sections and considering the
difference between data and our VDM calculations with $\sigma_{\phi
N}$=11~mb we estimate ${\tilde\Sigma}{<}$0.1~mb. In that case the
contribution from the two-step process is compatible with the direct
incoherent $\phi$-meson photoproduction and the coupled channel effect is
indeed sizable.

\subsection{Speculations}
Finally we would like to mention another possibility which is not
related to the $\phi$-meson propagation in nuclear matter and the
${\tilde\Sigma}$ transition but with incoherent $\phi$-meson
photoproduction at low energies. Recently~\cite{Sibirtsev11}
we investigated the role of
the cryptoexotic baryon with hidden strangeness, $B_\phi{=}udds{\bar
s}$, in $\phi$-meson production in proton-proton collisions close to
the reaction threshold. We found that the enhanced $\phi$-meson production
observed at COSY~\cite{Hartmann1} can be well explained by
an $B_\phi$-baryon excitation followed by the  $B_\phi{\to}\phi{N}$
decay. It is expected that these
pentaquark baryons have a narrow width and decay preferentially into the
$\phi{N}$, $K{\bar K}N$ or $YK$ channels, where $Y$ stands for ground-state
or excited hyperons~\cite{Landsberg1,Landsberg2}.
Experimental observations for the $B_\phi$ candidates were reported
in Refs.~\cite{Arenton,Aleev,Dorofeev1,Dorofeev2,Balatz,Antipov}.
The high-statistics study of Ref.~\cite{Antipov} of the
$\Sigma^0K^+$ mass spectrum indicates two exotic states with
$M = 1807{\pm}7$~MeV, $\Gamma = 62{\pm}19$~MeV and $M = 1986{\pm}6$~MeV,
$\Gamma = 91{\pm}20$~MeV.

One might expect that $B_\phi$-baryon can be excited in photon-nucleon
interaction. Because of its mass the $\gamma{p}{\to}\phi{p}$ reaction
would be sensitive to $B_\phi$ excitation at low photon energy. The
$B_\phi$ contribution might explain the SAPHIR-8 and SPRING-8
measurements~\cite{Barth,Mibe} of angular spectra in the
Gottfried-Jackson frame, which indicate that at low energies the
$\phi$-meson photoproduction is not governed by pomeron exchange.

Considering coherent and incoherent $\phi$-meson photoproduction from
nuclei we notice even more significant features. First, the coherent
photoproduction at low energies should not by dominated by
$B_\phi$-baryon excitation, since in that case the residual nucleus
differs from ground state. Incoherent $\phi$-meson
photoproduction at low energies might be dominated by $B_\phi$
excitation. Since the $B_\phi$-baryon is narrow, it decays outside the
nucleus and an effective distortion of the $\phi$-meson is given by the
distortion of $B_\phi$, which is compatible with and interaction of
other baryons in nuclear matter because of the light quark content of
the $B_\phi$-baryon. Therefore one should not be surprised by the result
shown in Fig.~\ref{spring1}.

\section{Conclusions}
We have analyzed coherent and incoherent $\phi$-meson photoproduction from
nuclei by applying the single and coupled channel optical model.

The data
on coherent $\phi$ photoproduction collected at Cornell~\cite{McClellan1} at
photon energies of 6.4 and 8.3~GeV can be well reproduced by a single
channel calculation taking into account the $\phi$-meson distortion
compatible with the $\phi{N}$ total cross section $\sigma_{\phi
N} =10$~mb. This result is in good agreement with the VDM analysis of
the forward $\gamma{p}{\to}\phi{p}$ differential cross section, which
indicates that $\sigma_{\phi N}{\simeq}$11~mb. Coherent
$\phi$-meson photoproduction shows little room for the coupled channel
effect due to the contribution from the $\omega {\to} \phi$ transition.

The data on incoherent $\phi$-meson photoproduction off various nuclei
collected at
SPRING-8~\cite{Ishikawa} at photon energies from 1.5 to 2.4~GeV can be
reproduced by the single channel optical model calculations only under
the assumption that the $\phi$-meson is substantially distorted in nuclei,
which corresponds to $23 {\le} \sigma_{\phi N} {\le} 63$~mb. This result is
in agreement with previous incoherent $\phi$-meson photoproduction data
analyses~\cite{Ishikawa,Cabrera,Munlich}. Moreover, we
found that taking into account the coupled channel effects, {\it i.e.}
assuming direct $\omega$-meson photoproduction followed by the
$\omega{N} {\to} \phi{N}$ transition as well as pion photoproduction
followed by the $\pi{N} {\to} \phi{N}$ scattering, it is possible to reproduce
the $A$-dependence measured at SPRING-8~\cite{Ishikawa}.

Although we
estimate the absolute rates for the contribution of these two
different intermediate states, it is difficult to draw a  final
conclusion. First, the SPRING-8 data~\cite{Ishikawa} are published
without absolute normalization. Second, the $t$-dependence of these
data are not given for all nuclei used in the measurements.
Such knowledge is essential for the evaluation of  incoherent
photoproduction within the coupled channel analysis, since each of the
two-step processes has an individual $t$-dependence, which can be used in
order to distinguish the intermediate states. In that sense more
precise data on incoherent $\phi$-meson photoproduction are necessary
for further progress.

We also discussed a very alternative (and probably speculative)
scenario that might occur only in
incoherent $\phi$-meson photoproduction but is not accessible in
the coherent reaction. The excitation of the cryptoexotic baryon with
hidden strange{\-}ness, called $B_\phi$, would result in an
$A$-dependence similar to that measured by SPRING-8~\cite{Ishikawa}.
However, the $B_\phi$-baryon could not be exited in coherent
photoproduction. Therefore measurements of the $A$-dependence of
coherent $\phi$-meson photoproduction from nuclei at low energies is
crucial for identification of the possible existence of such an
cryptoexotic baryon.

\subsection*{Acknowledgements}
We would like to thank   J. Haidenbauer, T. Nakano, A. Nogga for useful
discussions.  This work was partially  supported  by Deutsche
Forschungsgemeinschaft  through funds provided to the SFB/TR 16
``Subnuclear Structure of Matter''. This research is part of the \, EU
Integrated \, Infrastructure \, Initiative Hadron Physics Project under
contract  number RII3-CT-2004-506078. A.S. acknowledges support by the
JLab grant SURA-06-C0452  and the
COSY FFE grant No. 41760632 (COSY-085).

redpajama_set_name: RedPajamaArXiv


Basically similar to the Sagittario II, the Aerfer Ariete (Battering Ram) was built by Industrie Aeronautiche Meridionali (Aerfer), and represented the next step towards the development of the finally abortive Leone (Lion) mixed-power light interceptor fighter, which was being worked upon with the financial support of the US government. The Ariete had a deeper rear fuselage and, in addition to the Derwent 9, had an 821kg thrust Rolls-Royce Soar R.Sr 2 auxiliary turbojet, which improved overall performance. The Ariete prototype (MM 568) flew for the first time on 27 March 1958, but the entire project was later abandoned.
Concerning the abandon of the Aerfer fighter projects, rumours are of lobby activity by U.S.A. (for the F-86 Sabre) and by FIAT (for its G 91).
Very interesting plane. It had Hispano-Suiza HS-825 cannons which have scarce info on but I gathered enough.
The Ariete had 240 rounds in total in those 30mms.


HIDDEN Chambers of the Mausoleum on October-10-2014 in Crossroads Riverview Park by Riverview Recreation Park, LLC.
HIDDEN The Asylum at Coffin Creek on October-10-2014 in Crossroads Riverview Park by Riverview Recreation Park, LLC.
HIDDEN Nightmare Harvest Trail on October-10-2014 in Crossroads Riverview Park by Riverview Recreation Park, LLC.
HIDDEN Labyrinth of Lost Relics on October-10-2014 in Crossroads Riverview Park by Riverview Recreation Park, LLC.
HIDDEN Shady Hallow Hay Ride on October-10-2014 in Crossroads Riverview Park by Riverview Recreation Park, LLC.
HIDDEN Monali Thakur live in concert on October-04-2014 in Chabot College Auditorium by Bay Area Prabasi, Inc.


text:
Nova radio host retracts allegation True Story with Hamish & Andy was a stolen idea
By Áine Ryan| 2 years ago
Image: Nine
David 'Luttsy' Lutteral now says the idea for the show was not his.
The Nova radio host who claimed Andy Lee stole the idea for Nine's new series True Story with Hamish & Andy from him has now retracted his allegation.
In a statement made on his breakfast show Ash, Kip and Luttsy Thursday morning, David 'Luttsy' Lutteral said the following:
"Some things were said on our breakfast radio program on Monday about Hamish and Andy that were pretty serious allegations about the concept of their program true story being stolen from me after a conversation between Andy and me in New York in December 2014.
"I fully accept now that that was not the case. I've now seen the concept document from 2013 developed by Hamish and Andy's team for True Story. It is clear to me that they had conceived and documented the format for true story over a year before I met with Andy in New York.
"While I pitched a concept that had some similarities I accept that Hamish and Andy came up with their idea independently from mine. Wrongly accusing someone of stealing material is one of the most offensive things someone can do in our industry.
"I apologise to Hamish and Andy and their team for implying they took my idea."
Each week, True Story sees an everyday Australian tell Hamish and Andy an extraordinary story before the boys recreate with their comedic actor friends.
Ahead of True Story's premiere on Monday night, Luttsy took to his radio show and said that he told Andy, 36, about Cracking Yarns, a show he planned to pitch to TV networks when they were in a bar in New York.
"I've read the press release blurb for [True Story and it's] word-for-word the concept that I told Andy in 2014 in December," he told co-hosts Ashley Bradnam and Kip Wightman earlier this week.
Ash, Kip and Luttsy (R), Image: Nova
He then added that he and Ash had begun filming Cracking Yarns with Channel Nine, but that the show was never completed.
"Ash, you were part of the pilot we did," Luttsy said. "I'd half shot that pilot and then other things have taken over so I haven't actually completed it."
But Channel Nine were quick to deny the allegations, releasing a statement that same day.
Hamish (left) and Andy; Image: Nine
"Radio Karate [True Story's production company] have confirmed that the format for the program True Story with Hamish and Andy was conceived and was in development by Radio Karate, over a year before Andy and Luttsy met for a drink in New York."
True Story with Hamish & Andy marks the comedy duo's return to TV after three years and premiered to stellar ratings.
Their previous TV projects Gap Year and Caravan Of Courage were also both ratings successes.
Hamish and Zoe Foster Blake's son Sonny is perpetually grumpy
Hamish And Andy
Hamish Amp Andy
Sport Promotion: Ladbrokes members score more! Don't miss out! Gamble responsibly- ladbrokes.com.au

redpajama_set_name: RedPajamaCommonCrawl


With the PAC show coming up on Saturday I'm trying to not leave everything to the last minute this year! Hence much working and running around as I try to get rods finished for customers in time to allow me a day or two's rod testing (fishing) before the event.
One set of rods has allowed me to try a handle I've thought about for some time, and if you like full Duplon handles it looks pretty good. Kinda stealthy. Full Duplon is growing on me. I'm not ready to commit to it for any of my own rods just yet, though!
As well as my two new rods I'll have some other new and newish stuff on display and for sale at the show. It should be a good day.


This Pendant features a Fine Silver Hare and a AAA Quality Rainbow Moonstone.
New 20 mm Design Moon-gazing Hare Pendant.
Supplied with Sterling Silver bale for hanging on a Leather Thong or simple loop supplied with 18″ Sterling Silver Chain. Please tell me your preferred option.
The pendant features a Fine Silver sculpted Hare beneath the branch of a tree. Onto the bezel is set a AAA grade Moonstone. The metal work is suspended in front of a Black Lip Mother Of Pearl disk.
Price includes Sterling Silver 10 mm bale OR simple loop and Sterling Rope Chain.


text:
Q: Is there only a unique way to decompose a matrix as a series of multiplication of elementary matrix ? (RREF and invertible matrix) We know that for each given matrix, there exists only one unique matrix in row reduced echelon form.
We also know that the transformations of a matrix to another can be decomposed to a series of elementary matrices:
$$A=E_nE_{n-1}E_{n-2}\dots E_1 (P) \text{ (where P is the original matrix)}$$
As a result, I would like to ask:

*

*Does it exist only one way to transform a matrix to the RREF ?

*Is the matrix resulted from $E_nE_{n-1}E_{n-2}\dots E_1$ that transforms a matrix to its RREF unique?

We also know that to find the inverse of an invertible matrix, we can also apply a series of multiplication of elementary matrices.
In that case, is $E_nE_{n-1}E_{n-2}\dots E_1$ unique in finding the inverse matrix?

A: *

*The sequence of transformations is not unique. For example you can insert an operation, then undo it by applying the inverse of the operation.

*The matrix $E_nE_{n-1}\cdots E_1$ is not unique unless the original matrix $P$ is of full rank. For example, consider $P:=\begin{pmatrix}1&0\\1&0\end{pmatrix}$, whose RREF is $A:=\begin{pmatrix}1&0\\0&0\end{pmatrix}$. Try writing $A$ as the product $EP$, for $E:= \begin{pmatrix}a&b\\c&d\end{pmatrix}$. After expanding $EP$, you will find that the only constraints are $a+b=1$ and $c+d=0$. This means you have some freedom in selecting $a, b, c, d$.

*If $P$ has full rank, then the RREF $A$ is the identity matrix. So if $E$ satisfies the equation $A=EP$, then $E$ must be the inverse of $P$ and is therefore unique.

A: Try row reducing $\begin{pmatrix} 1 & 0 \\ -1 & 0 \end{pmatrix}$ in two ways: first, by just adding row 1 to row 2, and second, by swapping the rows, adding (the new) row 1 to (the new) row 2, and then scaling row 1 by -1. Pretty sure you get different products of $E$'s.
In more detail, consider the matrix $\begin{pmatrix} 1 & 0 \\ 1 & 1 \end{pmatrix}$ (implementing the first RREF) and the matrix product $\begin{pmatrix} -1 & 0 \\ 0 & 1 \end{pmatrix} \begin{pmatrix} 1 & 0 \\ 1 & 1 \end{pmatrix} \begin{pmatrix} 0 & 1 \\ 1 & 0 \end{pmatrix}$ (implementing the second). Are they the same?
As a metamathematical note, I came up with this example from a general intuition that the product of $E$s may depend on which rows you choose to use when clearing out entries from a given column.  Often you have some choice in that, and apparently it does make a difference.

redpajama_set_name: RedPajamaStackExchange


Starting a law career can be challenging. There's a lot of obstacles from just getting into college to scoring well on the LSAT. That's not even to mention applying for law school, law school, passing the bar, and working!! No matter where we are in the process having good support is so beneficial. We start when we say "I'm ready". Or sometimes we're not ready and start anyways! The idea is that this can be a network to find job opportunities, volunteer opportunities and support! This group will be network to help others with their process and get help for our own!


In 1987, the Bosque County Historical Commission published two volumes entitled Bosque County Cemetery Records. If the cemetery has been enumerated in the two-volume Bosque County Cemetery Records, the volume and page number is provided. Several cemeteries were relocated when the Brazos River was dammed up to form Lake Whitney. The two volumes of the Bosque County Cemetery Records list all persons buried in the cemeteries at the time of publication. The information also includes dates from the gravestones and, in some cases, the inscriptions from the gravestones. Although these volumes are now out-of-print, they are available for reference at the Bosque County Collection. The information contained in these volumes has been converted to an online database searchable by name. Search our online database.
The question often arises as to whether relatives can visit a cemetery on private land. State law grants the public certain rights for visitation during reasonable hours and for purposes associated with cemetery visits, but with conditions. Click here and read the "Access" section for more information.
Below are all the known cemeteries that exist today in Bosque County. If you think a cemetery is located in Bosque County but do not find it, check the tables at the bottom of this page for alternate/deprecated names and adjacent county cemeteries within a mile of Bosque County.
The HTC designation is an official recognition of family and community graveyards and was developed in 1998 to help protect historic cemeteries by recording cemetery boundaries in county deed records to alert present and future owners of land adjacent to the cemetery of its existence. The designation imposes no restrictions on private owners' use of the land adjacent to the cemetery or the daily operations of the cemetery. A cemetery is eligible for designation if it is at least 50 years old and is deemed worthy of recognition for its historical associations. The very nature of a cemetery being a landmark of a family's or community's presence is considered to validate the criteria of historical associations. Any individual, organization, or agency may submit a request for designation.
The Official Historic Texas Cemetery designation can be obtained through an application process with the Texas Historical Commission. Any individual, organization or agency may submit an application. To receive the designation, the applicant must show proof that the cemetery is at least 50 years old and provide precise information on its location. A processing fee of $25 is required. If a cemetery already has a Historical Marker, certain information requirements in the application can be waived. Once processed, the cemetery is recorded in the county deed records as a historic site and is eligible to display the Historic Texas Cemetery medallion. The medallion can be displayed by itself, as an addition to an already existing Historical Marker, or with a new interpretive plaque with text developed from the history. The cost of the medallion and plaques are additional but are not required for a cemetery to be designated as an Official Historic Texas Cemetery. The designation does not restrict in any way the public use or private owner's use of the land adjacent to the cemetery. Click here to find out more about the Historic Texas Cemetery program and download an application.


text:
ghacks.net
Firefox add-ons
AOL Buys Huffington Post for $315m
Mike Halsey MVP
Updated • Feb 8, 2011
The Huffington post has now confirmed that its been bought by AOL for $315 million. The website, which was launched in 2005, is essentially a news aggregator featuring coverage of politics, media, business, entertainment, lifestyle, world news and so on.
AOL is still relying on revenues from existing subscribers to it's dial up services. It's been reported that 80% of its current revenues still come from this source, providing the company with about $244 million every year. The company is clearly looking at new sources of income however and the Huffington Post is one it's decided will make a good acquisition.
In a statement they said...
The transaction will create a premier global, national, local, and hyper-local content group for the digital age - leveraged across online, mobile, tablet, and video platforms. The combination of AOL's infrastructure and scale with The Huffington Post's pioneering approach to news and innovative community building among a broad and sophisticated audience will mark a seminal moment in the evolution of digital journalism and online engagement.
AOL also owns many other popular websites including the tech websites TechCrunch and Engadget. Huffington have said "By uniting AOL and The Huffington Post, we are creating one of the largest destinations for smart content and community on the Internet. And we intend to keep making it better and better."
It can be certain that this acquisition will generate much needed additional revenue for AOL, though how many years it will take to recoup such a huge investment remains to be seen.
AOL has seen many financial scares, purchases and sales in the last few years. The company is no doubt looking with this aquisition to stabilise its financial future.
About Mike Halsey MVP
Mike Halsey is a Microsoft MVP (Windows Expert) and the author of "Troubleshooting Windows 7 Inside Out" from Microsoft Press, "Office 365 Security Essentials" and several forthcoming books about Windows 8. He is a recognised Windows expert having been awarded a Microsoft MVP (Most Valuable Professional) certification in 2011. You can follow Mike on Facebook, Twitter, Google+ or on his own website The Long Climb
View all posts by Mike Halsey MVP →
Startpage Search Engine launches Privacy Protection extension
You may soon display vertical tabs in Microsoft Edge on the right side
Audible app for Windows has been discontinued, company advises users to switch to the Cloud Player or mobile apps
A bug in Vivaldi browser disables the forward and back buttons if you open a new window
Bittorrent client qBittorrent 4.4.0 released with v2 torrent support
Microsoft Edge 97 released: here is what is new
Previous Post: « IBM Celebrates 100 Years
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Ali said on February 7, 2011 at 5:29 pm
I donno whether this acquisition is good or bad news for techies!!!
Avatar X said on February 8, 2011 at 12:20 am
"The Huffington Post also owns many other popular websites including the tech websites TechCrunch and Engadget. "
Aol also owns… is what you meant.
Martin said on February 8, 2011 at 12:23 am
Thanks, corrected it.
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Brave acquires Tailcat search engine; will offer search results without profiling users
Brave browser adds native support for uBlock and Fanboy annoyances lists and social list
Brave reveals why it is disabling Google's FLoC in the browser
DuckDuckGo Extension blocks Google FLoC in latest update
Brave Search Beta is now available publicly
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UUSC staff testify before the Joint Committee on the Judiciary at the Massachusetts State House in support of H.3033, a bill designed to end 287(g) agreements in the state.
On May 8, UUSC Vice President and Chief Program Officer Rachel Freed testified on a panel before the Joint Committee on the Judiciary at the Massachusetts State House in support of H.3033, a bill designed to end 287(g) agreements in Massachusetts by preventing state and local funds from being used to enforce federal immigration laws. The panel supporting H.3033 was organized by the Massachusetts Immigrant and Refugee Advocacy Coalition (MIRA) and included UU Mass Action Executive Director Laura Wagner and Bishop Felipe Teixeira of the Franciscan Order of Saint Joseph Cupertino. Support for H.3033 was high with over 30 speakers supporting the bill and only three in opposition, including Bristol County Sheriff Hodgson who infamously offered to send his inmates to build the U.S.-Mexico border wall without pay.
The hearing came one day after Texas Governor Greg Abbott signed SB4 into law, a vehemently anti-immigrant bill criminalizing cities that want their law enforcement to focus on "safety" and not immigration. SB4 prohibits Texas law enforcement from practicing "sanctuary" policies and allows authorities to question someone's immigration status based on racial profiling. The bill is now facing lawsuits from civil rights organizations.
287(g) agreements are one of the main ways that local and state law enforcement agencies become empowered to serve as an arm of Immigration and Customs Enforcement (ICE) and are granted authority to identify and hold undocumented immigrants for deportation. These agreements deputize police and sheriff officers to act as immigration agents and provide them with minimal training before authorizing them to perform immigration-related duties. . Implementation of the program is entirely funded by the local agencies themselves rather than the federal government.
Passing H.3033 and ending 287(g) agreements is an important first step for the state, but also not enough. This is why many Massachusetts communities are rallying behind immigrants and are focusing on getting involved at the local level.
UUSC continues to work in coalition in Massachusetts to support these efforts as well as to pass groundbreaking state legislation like the Safe Communities Act (S.1305 and H.3269). The Safe Communities Act would set a new standard for pro-immigrant state legislation. It both goes further to restrict local agents' participation in immigration enforcement and also prohibits state law enforcement agencies and the Mass. Registry of Motor Vehicles from allowing federal access to their data, limiting their ability of the federal government to use that data for the purpose of a Muslim registry or another tracking system based on religion or national origin.
Update as of May 24, 2017: H.3033 was reported out favorably from the Joint Committee but the planned vote was "indefinitely postponed" today. UUSC is closely following the legislation to see where Massachusetts lands.


text:
Cinema
 Faithful – film del 1910 diretto da David Wark Griffith
 Faithful – film del 1936 diretto da Paul L. Stein
 Infedeli per sempre (Faithful) – film del 1996 diretto da Paul Mazursky

Musica
 Faithful – album di Todd Rundgren del 1976
 Faithful – album di Dusty Springfield del 2015

Letteratura
 Faithful – libro di Stephen King del 2004

Pagine correlate
Faithfull

redpajama_set_name: RedPajamaWikipedia


text:
Caratteristiche tecniche
É un centrale di centrocampo.

Carriera

Club
Inizia la carriera nelle giovanili del  di Montevideo, che nel 2005 lo cede al , in Spagna; dopo una stagione nella terza divisione iberica lascia la squadra e va a giocare al Victoria de Tazacorte in Tercera División (la quarta serie spagnola). A fine stagione lascia la Spagna per andare a giocare in Italia alla Sporting Genzano, nel campionato lucano di Eccellenza, che vince ottenendo la promozione in Serie D. Dopo una stagione lascia la squadra e torna in Uruguay, al , con cui nella stagione 2009-2010 disputa 7 partite nella massima divisione uruguaiana. Tra il gennaio del 2010 ed il luglio del 2012 veste invece la maglia del , formazione della prima divisione venezuelana. Dal luglio del 2012 al gennaio del 2013 è invece ancora in patria, questa volta al .

Nazionale
Nel 1999 ha partecipato con la Nazionale Under-17 al campionato sudamericano di categoria.

Palmarès

Club

Competizioni regionali

Sporting Genzano: 2007-2008

Note

Collegamenti esterni


text:
What is 305 Hours in Seconds?
Hours to Seconds
305 hr in s
305 Hours =
1098000 Seconds
Convert 305 Hours to Seconds
To calculate 305 Hours to the corresponding value in Seconds, multiply the quantity in Hours by 3600 (conversion factor). In this case we should multiply 305 Hours by 3600 to get the equivalent result in Seconds:
305 Hours x 3600 = 1098000 Seconds
305 Hours is equivalent to 1098000 Seconds.
How to convert from Hours to Seconds
The conversion factor from Hours to Seconds is 3600. To find out how many Hours in Seconds, multiply by the conversion factor or use the Time converter above. Three hundred five Hours is equivalent to one million ninety-eight thousand Seconds.
Definition of Hour
An hour (symbol: h; also abbreviated hr.) is a unit of time conventionally reckoned as 1⁄24 of a day and scientifically reckoned as 3,599–3,601 seconds, depending on conditions. The seasonal, temporal, or unequal hour was established in the ancient Near East as 1⁄12 of the night or daytime. Such hours varied by season, latitude, and weather. It was subsequently divided into 60 minutes, each of 60 seconds. Its East Asian equivalent was the shi, which was 1⁄12 of the apparent solar day; a similar system was eventually developed in Europe which measured its equal or equinoctial hour as 1⁄24 of such days measured from noon to noon. The minor variations of this unit were eventually smoothed by making it 1⁄24 of the mean solar day, based on the measure of the sun's transit along the celestial equator rather than along the ecliptic. This was finally abandoned due to the minor slowing caused by the Earth's tidal deceleration by the Moon. In the modern metric system, hours are an accepted unit of time equal to 3,600 seconds but an hour of Coordinated Universal Time (UTC) may incorporate a positive or negative leap second, making it last 3,599 or 3,601 seconds, in order to keep it within 0.9 seconds of universal time, which is based on measurements of the mean solar day at 0° longitude.
Definition of Second
The second (symbol: s) (abbreviated s or sec) is the base unit of time in the International System of Units (SI). It is qualitatively defined as the second division of the hour by sixty, the first division by sixty being the minute. The SI definition of second is "the duration of 9 192 631 770 periods of the radiation corresponding to the transition between the two hyperfine levels of the ground state of the caesium 133 atom". Seconds may be measured using a mechanical, electrical or an atomic clock. SI prefixes are combined with the word second to denote subdivisions of the second, e.g., the millisecond (one thousandth of a second), the microsecond (one millionth of a second), and the nanosecond (one billionth of a second). Though SI prefixes may also be used to form multiples of the second such as kilosecond (one thousand seconds), such units are rarely used in practice. The more common larger non-SI units of time are not formed by powers of ten; instead, the second is multiplied by 60 to form a minute, which is multiplied by 60 to form an hour, which is multiplied by 24 to form a day. The second is also the base unit of time in other systems of measurement: the centimetre–gram–second, metre–kilogram–second, metre–tonne–second, and foot–pound–second systems of units.
Using the Hours to Seconds converter you can get answers to questions like the following:
How many Seconds are in 305 Hours?
305 Hours is equal to how many Seconds?
How to convert 305 Hours to Seconds?
How many is 305 Hours in Seconds?
How much is 305 Hours in Seconds?
How many s are in 305 hr?
305 hr is equal to how many s?
How to convert 305 hr to s?
How many is 305 hr in s?
What is 305 hr in s?
How much is 305 hr in s?
What is 305 Hours in other Time units?
305 Hours in Days
305 Hours in Months
305 Hours in Years
305 Hours in Milliseconds
305 Hours in Nanoseconds
305 Hours in Weeks
Conversions similar to 305 Hours to Seconds
306 Hours in Seconds
Previous Hours to Seconds conversions
80 Hours in Seconds
1695 Hours in Seconds
138 Hectares in Square Yards
459 Knots in Meters/Second
1195 Cubic Feet in Liters
453 Short Tons in Kilograms
539 Centimeters in Feet
472 Feet in Meters
1158 Centimeters in Millimeters
713 Hectares in Square Meters
1353 Milligrams in Pounds
311 Square Feet in Square Meters
288 Kilometers in Yards
464 Days in Minutes
1430 Years in Nanoseconds


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Cracking down on backdoor listing
Written by: Gary Lock, Ruth Lau and Eugene Lau.
In response to concerns on rampant "shell activities" involving backdoor structures in recent years, the Hong Kong Stock Exchange (the "HKEx") published a consultation paper in June 2018 on backdoor listing and continued listing criteria (the "Consultation Paper").
After a rather prolonged deliberation the HKEx finally published the conclusions (the "Conclusions"), with new rules (the "Rules") in July 2019. The Rules will take effect in October 2019.
New Rules relating to Backdoor Listing
The following major changes will be implemented:
codifying the following six RTOs assessment criteria in Guidance Letter GL78-14 as notes to Rules 14.06B:
the size of the acquisition or series of acquisitions relative to the size of the issuer;
a fundamental change in the issuer's principal business;
the nature and scale of the issuer's business before the acquisition or series of acquisitions;
the quality of the acquisition targets;
change in control or de facto control of the issuer; and
series of transactions or arrangements to list the acquisition targets;
Rules 14.92 and 14.93 are modified to restrict any material disposal (or a disposal by way of distribution in specie that amounts to a material disposal) of an issuer's existing business at the time of or within 36 months after a change in control, unless (i) its remaining business or (ii) the assets acquired from the new controlling shareholder and any other persons, would meet the requirements under Rule 8.05;
codifying the "extreme VSA" in Guidance Letter GL78-14 as Rule 14.06C, and renaming this category of transaction as "extreme transaction" and issuers would only be able to rely on this provision if it (a) has been operating a principal business with substantial size which will continue after the transaction; or (b) has been under the control of the same person for a long period (normally not less than three years); and
codifying Guidance Letter GL84-15, whereby the HKEx may ban large scale issue of new securities if the proceeds are used to acquire new or greenfield businesses that are expected to be substantially larger than the issuer's existing business.
Modified Rules relating to Continued Listing Criteria
The current Rule 13.24, which requires an issuer to have directly or indirectly, sufficient level of operations OR have assets of sufficient value to warrant the continued listing of the issuer's securities will be modified. Under the new Rule 13.24:
an issuer is required to have directly or indirectly, a business with sufficient level of operations AND assets of sufficient value to support its operations to warrant the continued listing of the issuer's securities; and
proprietary trading and/or investment in securities by an issuer and its subsidiaries (other than an issuer which is an investment company listed under Chapter 21 or proprietary securities trading and/or investment activities carried out in the ordinary and usual course of business by a member of an issuer's group that is a banking company, an insurance company or a securities house) are normally excluded when considering whether the issuer can meet Rule 13.24.
A transitional period of 12 months from the effective date of the Rule amendments will apply to listed issuers that do not comply with the new Rule 13.24.
Other Rules Amendments
Other new or modified other Rules have also been introduced by the Consultation Paper and adopted (with modifications) in the Conclusions, which are relevant for ongoing listing compliance all the issuers:
the revenue exemption under Rule 14.04(1)(g) for purchases and sales of securities will only apply to cases where they are (i) conducted by banking companies, insurance companies and securities houses; and (ii) conducted within their ordinary and usual course of business by those banking companies, insurance companies and securities houses. For any other cases, including securities trading which were previously allowed under Listing Decision LD53-2, will generally be caught as notifiable transactions;
the issuers are required to disclose following details of securities investment that represents 5% or more of the total assets in the annual report:
the name and principal business of the underlying company, the number and percentage of shares held and the investment costs;
the fair value of each investment as at the year end date and its size relative to the issuer's total assets;
the performance of each investment during the year, including any realized and unrealized gain or loss and any dividend received; and
a discussion of the issuer's strategy for the significant investments;
new Rule 14.36B, which applies in cases where the issuer acquires a company or business from a person and that person guarantees the profits or net assets or other matters regarding the financial performance of the company or business. In such cases the issuer must issue update announcements if there are any subsequent changes or deviation in performance; and
for announcements under Chapters 14 and 14A:
any notifiable transaction announcement to expressly state the identity of the counterparty (a general description will no longer suffice); and
any connected transaction announcement to disclose on the identities and activities of the parties to transactions and of their ultimate beneficial owners.
Clients are strongly advised to seek advice at an early stage when contemplating any merger and acquisition activities of listed companies in Hong Kong as a platform to expand their businesses. Please reach out to a member of our team should you require further information in relation to any of the above.
Gary Lock
M +852 9819 2328
Ruth Lau
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Home > National Railway Museum > England > Cheshire & Staffordshire
Framed Print of Newton, Cheshire, London & North Western Railway, 1848
> Transport
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Newton, Cheshire, London & North Western Railway, 1848
Lithograph, drawn and lithographed by the American-born artist Arthur Fitzwilliam Tait (1819-1905), showing a haywain being pulled along a street with a railway viaduct in the background. The London & North Western Railway was created in 1846 from the amalgamation of the Grand Junction Railway, the London & Birmingham Railway and the Manchester & Birmingham Railway. Printed & published by Bradshaw & Blacklock, London & Manchester.
Lithograph, drawn and lithographed by the American-born artist Arthur Fitzwilliam Tait (1819-1905), showing a haywain being pulled along a street with a railway viaduct in the background. The London & North Western Railway was created in 1846 from the amalgamation of the Grand Junction Railway, the London & Birmingham Railway and the Manchester & Birmingham Railway. Printed & published by Bradshaw & Blacklock, London & Manchester
We are proud to offer this print in collaboration with National Railway Museum
© Please read our licence terms. All digital images must be destroyed unless otherwise agreed in writing.
Cheshire Lnwr Horses Carts Horse Drawn Vehicles Haywains Towns Streets V , Newton , Railway
> National Railway Museum > England > Cheshire & Staffordshire
> National Railway Museum > Images Dated > 2003 > February > 24 Feb 2003