text:
\section{Introduction}

Matrix theory \cite{BFSS} purports to be a complete, non-perturbative
formulation of M theory. Since a great deal is known about the
physics of M theory in various corners of moduli space, much
effort has recently been directed towards verifying that such
physics can be recovered from Matrix theory. In this paper we will
be primarily interested in studying the description of D-branes that
emerges when Matrix theory is compactified on a circle, yielding the
type IIA theory. Some salient features of D-branes in IIA theory which
one would like to obtain from Matrix theory include the following: there
exist Dp-branes for p = 0,2,4,6,8; the low energy dynamics of k parallel
Dp-branes is described by a supersymmetric p+1 dimensional U(k) gauge
theory; the (not necessarily low energy) dynamics of a single D-brane is
described by a Born-Infeld type action. In addition, one knows the
supergravity fields produced by D-branes and so also the corresponding
small angle scattering amplitudes of several such objects.

Banks, Seiberg, and Shenker \cite{BSS}, and S.-J. Rey \cite{SJR},
took some first steps towards
deriving the effective actions of D-branes from Matrix theory. They
identified matrix assignments corresponding to D-branes by identifying
the appropriate central charges in the 11 dimensional light cone gauge
supersymmetry algebra. Then by analyzing the fluctuations around such
backgrounds and replacing large N commutators by Poisson brackets, they
were able to recover the general structure of the known effective actions
to quadratic order in fields. Here, our goal is similar, but we wish to go
beyond quadratic order and to keep careful track of numerical factors. To
do so successfully, we found it necessary to replace matrix commutators not
by Poisson brackets but rather by the commutators of covariant derivatives,
much as one does when considering toroidal compactification. By so doing,
we are able to obtain gauge invariant actions which precisely reproduce
the  fluctuations of the Born-Infeld action in the presence of a
large background magnetic field.

There have been a number of studies comparing D-brane scattering
amplitudes obtained from Matrix theory and from supergravity. On the Matrix
theory side, the procedure involved computing the effective action of a
finite N matrix configuration, and then extrapolating to large N. Strictly
speaking, this procedure is inconsistent as the backgrounds require that
certain finite N matrices have a commutator proportional to the identity,
even though such matrices cannot exist. In our approach, we avoid this
problem by taking $N \rightarrow \infty$ from the outset. As a specific application,
we consider the scattering of a D0-brane from a configuration
composed purely of D6 and D0 branes \cite{WT}, which has not
been studied before. We find
complete agreement at the one loop level between Matrix theory and
supergravity.

The remainder of this paper is organized as follows. In section 2
we rewrite the Matrix theory action in a manner suitable for the study of
D-branes. Sections 2.1 and 2.2 focus on the
effective action for D2-branes, and
section 2.3 on the effective action for D4-branes. In section 3 we compute the
potential between a D0-brane and a D6+D0 configuration, and in section 4 we
discuss some of our results.

\bigskip

\section{Fluctuations of branes in Matrix theory}

The action governing Matrix theory is gotten by
dimensionally reducing the action of 10 dimensional
Super Yang-Mills theory to 0+1 dimensions.
In string units ($2\pi \alpha' =1$) the
bosonic part of the Lagrangian is\footnote{following \cite{BFSS}, Appendix B}
\begin{equation}
  {\cal L}_B = {\rm Tr} \ L_B \ ; \ L_B = \frac{T_0}{2}
 \{ (D_0X_I)^2 + \frac{1}{2} [X_I,X_J]^2 \}
\end{equation}
where $T_0$ is the D0-brane ``tension''
$$
T_0 = \frac{1}{\sqrt{\alpha'} g} = \frac{\sqrt{2\pi}}{g} \ ,
$$
the covariant derivative $D_0$ is
$$
D_0 = \partial_t - i[A_0,\ \cdot \  ]
$$
and $I=1,2,\ldots ,8,9$. A p-brane background is described by
\begin{eqnarray}
   X_r &=& U_r \ ; \  r=1,2,\ldots ,p \\
   X_i &=& 0   \ ; \ i=p+1,\ldots ,9
\end{eqnarray}
where $U_r, r=1,\ldots ,p$ are certain matrices to
be specified later.

Fluctuations around this background are denoted by $A_r,\phi_i$,
\begin{equation}
  X_r = U_r + A_r
\label{axar}
\end{equation}
\begin{equation}
  X_i = \phi_i \ .
\end{equation}
Following Banks, Seiberg and Shenker \cite{BSS}, we
substitute the above expansions into the Lagrangian $L_B$, and
then regroup and rename the terms so that we arrive at the following
form:
\begin{equation}
L_B = \frac{T_0}{2} \{ -\frac{1}{2} (F_{\mu \nu})^2 + (D_{\mu}\phi_i)^2
      +\frac{1}{2} [\phi_i,\phi_j ]^2 + i[U_r,U_s]F_{rs}
          + \frac{1}{2} [U_r,U_s]^2 \} \ ,
\label{basicL}
\end{equation}
where $\mu,\nu = 0,1,\ldots ,p; r,s=1,\ldots ,p$ and
\begin{eqnarray*}
 F_{0r} &=& -F_{r0} = \partial_0 A_r + i[U_r,A_0] - i[A_0,A_r] \\
 F_{rs} &=& -i[U_r,A_s] + i[U_s,A_r] -i[A_r,A_s] \\
 D_0\phi_i &=& \partial_0\phi_i -i[A_0,\phi_i] \\
 D_r\phi_i &=& -i[U_r,\phi_i] -i[A_r,\phi_i] \ .
\end{eqnarray*}
(In the above, $(D_{\mu}\phi_i)^2 = (D_0\phi_i)^2 - (D_r\phi_i)^2$ etc.)

So far, we have not done anything other than reorder the terms and
give them new names. Now we try to interpret the result
in the context of some particular p-brane backgrounds.

\bigskip

\subsection{Infinite membrane backgrounds (p=2)}

\bigskip

The 11 dimensional SUSY algebra admits central charges corresponding to the
presence of membranes. Banks, Seiberg and Shenker \cite{BSS} computed the
central charges starting from the Matrix theory action
and found\footnote{with the normalization corresponding
to conventions in this paper}
\begin{equation}
    Z_{rs} = -\frac{i}{2\pi} {\rm Tr} [X_r,X_s] \ .
\end{equation}
It follows immediately that $Z_{rs}$ vanishes for finite $N$. On the other
hand, it has recently been proposed by Susskind \cite{Nfin} that the
finite $N$ version of Matrix theory is to be interpreted as describing a
finite longitudinal momentum sector of M theory quantized in light cone
gauge. The vanishing of $Z_{rs}$ at finite $N$ can be understood in this
light, for a membrane carrying finite momentum must necessarily be compact
and so carry no net central charge.

Ref. \cite{BFSS} discussed a formal
method for constructing membrane backgrounds in the $N \rightarrow \infty$ limit. The
construction uses
canonical variables $Q,P$ obeying the commutation relation
\begin{equation}
     [Q,P] = \frac{2\pi i}{N} \ .
\end{equation}
Since this relation cannot be satisfied at finite $N$, we will instead
take the $N \rightarrow \infty$ limit in terms of the rescaled variables \cite{AB}
\begin{equation}
    U_1 = Q\sqrt{Nz_{12} } \ ; \ U_2 = P\sqrt{Nz_{12} }  \ .
\end{equation}
Taking the spectrum of $P,Q$ to go from 0 to $2\pi$, the area of the membrane
is $A = (2\pi )^2 N z_{12}$, becoming infinite in the $N \rightarrow \infty$ limit.
The commutation relation
\begin{equation}
  [U_1,U_2] = 2 \pi i z_{12}
\label{infbrane}
\end{equation}
can be represented by differential operators acting on a space of functions.
More formally, the $N$ dimensional vector space $V_N$ on which the matrices
$X$ act will be replaced by an infinite dimensional space
$V_{\infty}$ of functions on the membrane worldvolume. The membrane background
$U_1,U_2$ is represented by differential operators acting on $V_{\infty}$,
and fluctuations will be represented by elements of $V_{\infty}$,
{\em i.e.}, functions on the membrane worldvolume.

A simple representation of $U_{1,2}$ found in the literature
consists of taking
\begin{equation}
   U_1 = 2\pi i z_{12} \partial_y \ \ ; U_2 = y
\end{equation}
in the $N\rightarrow \infty$ limit. As Aharony and Berkooz \cite{AB} have
pointed out, a cosmetic flaw of this
representation is that a membrane
carries two spatial coordinates whereas only one is
manifest in the above equation.

There exists, however, a more ``natural'' representation than
the one given above. Membranes carry a charge, which
in Matrix theory
arises from a U(1) subgroup of the U(N) symmetry, or in the continuum
limit, the U(1) subgroup of U($\infty $) which is isomorphic with the
infinitesimal area preserving diffeomorphisms of the membrane.
Specifically, the membrane charge density $2\pi z_{12}$ is
associated with a U(1) magnetic field living on the membrane world volume.
In ten dimensions the boosted membrane corresponds to a D2-brane with a
large background magnetic field $f_{12}$ on its worldvolume, related to
the density $\sigma_0$ of D0-branes bound to the D2-brane by \cite{Town}:
\begin{equation}
       \sigma_0 = \frac{1}{2\pi} f_{12} \ .
\end{equation}
Since the D0-brane density is
\begin{equation}
       \sigma_0 = \frac{N}{A} =   \frac{1}{(2\pi )^2 z_{12}} \ ,
\label{d0density}
\end{equation}
we find that the magnetic field is given by
\begin{equation}
           f_{12} = \frac{1}{2\pi z_{12}} \ .
\label{magnfield}
\end{equation}
Let ${\bf a} \equiv (a_1,a_2)$ be the background U(1) vector potential
corresponding to the magnetic field: $f_{12} = \nabla \times {\bf a}$. We choose
\begin{equation}
    a_1 = -\frac{1}{2} f_{12} x_2 \ \ , \ \ a_2 = \frac{1}{2} f_{12} x_1  \ \ .
\label{backgr}
\end{equation}
Then, a representation of $U_{1,2}$, in which both of the membrane
coordinates and the background magnetic field are manifest, is given by
\begin{equation} \begin{array}{l}
  U_1 \leftrightarrow 2\pi z_{12} \ (i\partial_{x_1} + a_1(x_1,x_2)) \\
  U_2 \leftrightarrow 2\pi z_{12} \ (i\partial_{x_2} + a_2(x_1,x_2)) \end{array} \ .
\label{covder}
\end{equation}
This representation satisfies the commutation relation (\ref{infbrane}).
To avoid confusion, let us point out that although expressions
similar to (\ref{covder}) appear in
the context of toroidal compactification \cite{GRT},
here the motivation and the interpretation
are quite different.
We have not T-dualized anything,
the two coordinates $x_1,x_2$ parametrize the infinite membrane,
$(x_1,x_2) \in R^2$.

All other $N \times N $ matrices are represented by functions on the membrane
worldvolume:
\begin{eqnarray}
 \phi_i &\leftrightarrow & \phi_i (x_1,x_2) \\
    A_0 &\leftrightarrow & A_0(x_1,x_2) \nonumber \ .
\label{others}
\end{eqnarray}
(We have suppressed the dependence on the worldvolume time coordinate.)
For the components $A_r,\ r=1,2$ we will choose
\begin{equation}
  A_r \leftrightarrow 2\pi z_{12} \  A_r(x_1,x_2)  \ .
\label{aar}
\end{equation}
With this normalization, (\ref{axar}) becomes
\begin{equation}
 X_r \leftrightarrow 2\pi z_{12} \ [i\partial_{x_r} + a_r(x_1,x_2)
                                               + A_r(x_1,x_2)] \ ,
\end{equation}
and we see that $A_{\mu}(x_1,x_2)$ then has the proper interpretation
as the fluctuation around the background (\ref{backgr}).

In the $N \rightarrow \infty$ limit, the trace operation is replaced by
integration over the spatial membrane worldvolume coordinates $x_1,x_2$:
\begin{equation}
     {\rm Tr} \leftrightarrow \sigma_0 \int \ dx_1dx_2 \ \ ,
\label{trace1}
\end{equation}
where the normalization factor
$\sigma_0$ is included in
order to preserve the interpretation of the rank
of the matrices as the number of D0-branes $N=Tr {\bf 1}_N$; we
represent the unit matrix ${\bf 1}_N$ by 1.

Finally, the matrix commutators
which involve $U_r$ become commutators of operators
and functions, {\em e.g.}
\begin{equation}
     [U_r,A_0] \leftrightarrow (2\pi z_{12})
                              [i\partial_r + a_r(x_1,x_2) , A_0(x_1,x_2)] \ ,
\end{equation}
and the matrix commutators which do not involve $U_r$ become commutators
of functions, {\em e.g.}
\begin{equation}
     [\phi_i,\phi_j] \leftrightarrow  [\phi_i(x_1,x_2),\phi_j(x_1,x_2)] \ .
\label{commutator}
\end{equation}
In the case of a single membrane, these will be zero.

Now we can see what happens to $L_B$. It becomes a 2+1 dimensional
Lagrangian density with the terms
$$
\begin{array}{lcccr}
 F_{0r} & = & \partial_0 A_r +i[U_r, A_0] - i[A_0,A_r]
    & \leftrightarrow & (2\pi z_{12} )\ (\partial_0 A_r(x) - \partial_r A_0(x)) \\
F_{12} & = &  -i[U_1,A_2] +i[U_2,A_1] - i[A_1,A_2]
  & \leftrightarrow & (2\pi z_{12} )^2 \  (\partial_1 A_2(x) - \partial_2 A_1(x)) \\
D_0\phi_i & = & \partial_0 \phi_i - i[A_0,\phi_i]
 & \leftrightarrow & \partial_0 \phi_i(x) \\
D_r\phi_i & = &  -i[U_r,\phi_i] - i[A_r,\phi_i]
 & \leftrightarrow & (2\pi z_{12} ) \ (\partial_r \phi_i (x))
\end{array}
$$
We find
\begin{equation}
  {\cal L}_B = {\rm Tr} L_B \leftrightarrow
    \sigma_0 \int d^2x \ \frac{T_0}{2} \{ -\frac{1}{2}
     (F_{\mu \nu} F^{\hat{\mu} \hat{\nu}}) +
    \partial_{\mu} \phi_i \partial^{\hat{\mu}} \phi_i
    -2 (2\pi z_{12} )^3 F_{12} - (2\pi z_{12} )^2 \} \ ,
\label{U(1)L}
\end{equation}
where $F_{\mu \nu} = \partial_{\mu} A_{\nu} - \partial_{\nu} A_{\mu}$, and
the hatted upper indices are raised with the metric
\begin{equation}
 \hat{\eta}_{\mu\nu} = {\rm diag}\ (1, -\frac{1}{(2\pi z_{12} )^2},
                                     -\frac{1}{(2\pi z_{12} )^2}) \ .
\label{ppmetric}
\end{equation}
As a check, using the last term we can work out the tension of the membrane
to be
\begin{equation}
    T_2  = \frac{1}{2\pi} T_0
\label{tension}
\end{equation}
which is correct.
Notice that a key feature of our representation
in the $N \rightarrow \infty$ limit is the vanishing of commutators such
as (\ref{commutator}). This is in contrast to the approach in \cite{BSS},
where the authors represented the commutators of matrices
by Poisson brackets. Such a representation yields  nonvanishing
contributions such as
$$
  \{A_r,A_s \}
$$
to the $F_{rs}$ component of the field strength, which is cumbersome from
the D2-brane point of view where one expects to obtain
a U(1) symmetry. This puzzle seems to be related to the distinction
between infinite and finite membranes; for
discussion, see \cite{AB}.
Note also that even if the commutators vanish for a single infinite
membrane, we will obtain nonvanishing commutators
later when we discuss the case of multiple membrane backgrounds.

It is interesting to examine the relation between the effective action
(\ref{U(1)L}) which was derived from Matrix theory, and the analogous
Born-Infeld action for a D2-brane in IIA theory. The latter is
\begin{equation}
  L_{BI} = -T_2 \int \! d^2x \sqrt{\det [\eta_{\mu \nu} + F_{\mu \nu}
-\partial_\mu \phi_i \partial_\nu \phi_i]} \ ,
\label{BI}
\end{equation}
We recall that boosting to the infinite momentum frame in the eleven
dimensional description corresponds in ten dimensions to turning on a large
magnetic field on the worldvolume of the D2-brane.  We therefore make the
replacement $F_{12} \rightarrow f_{12}+F_{12}$, where
$f_{12} = {1 \over {2\pi z_{12}}}$ as in (\ref{magnfield}), and
expand $L_{BI}$ for large $f_{12}$. To quadratic order in fluctuations we find
\begin{eqnarray}
 L_{BI} &=&  -T_2 \int \! d^2x \left\{ \frac{1} {2 \pi z_{12}}
                                      +F_{12} \right\} \\
\mbox{} &-& {T_2 \over 2} \int \! d^2x  \left\{ (2\pi z_{12})
 + (2\pi z_{12})^2 F_{12} + {1 \over (2\pi z_{12})} {1\over 2}
           F_{\mu\nu}F^{\hat{\mu}\hat{\nu}}
     - {1 \over (2\pi z_{12})} \partial_{\mu} \phi_i \partial^{\hat{\mu}} \phi_i\right\}
       \nonumber \ .
\label{expandBI}
\end{eqnarray}
Again, upper indices are raised with the metric (\ref{ppmetric}).
To compare with Matrix theory the expression in the first set of  braces
should be subtracted according to $H_{IMF}=H-p_{11}$.  Then, using
$T_2=T_0/2\pi$ and (\ref{d0density}), comparison
of $L_{BI}$ with (\ref{U(1)L}) shows complete agreement except
for a factor of $1/2$ multiplying the term linear in $F_{12}$.  This term is
a total derivative and does not appear to  be significant.

The action (27) represents the starting point for a calculation
of Polchinski and Pouliot \cite{PP} involving M-momentum transfer between
membranes. (Related discussion can be found in \cite{DKM,BFSS2}.)
There it was assumed that the action could be obtained directly from Matrix
theory; here we have shown explicitly how this can be accomplished.

Consider now a background configuration of $k$ parallel
infinite membranes in the transverse directions $X_1,X_2$. At finite
$N$, this is represented by block diagonal $kN\times kN$ matrices,
$X_1$ has $k$ copies of the ``$N \times N $ matrix'' $Q$ in the diagonal, and $X_2$
has $k$ copies of $P$. Correspondingly, for $k$ infinite membranes
we take
\begin{eqnarray}
     U_1 &\leftrightarrow & 2\pi z_{12} (i\partial_1 + a_1) \otimes {\bf 1}_k \\
     U_2 &\leftrightarrow & 2\pi z_{12} (i\partial_2 + a_2) \otimes {\bf 1}_k
\end{eqnarray}
where ${\bf 1}_k$ is the unit $k\times k$ matrix. Thus,
\begin{equation}
   [U_1,U_2] = 2\pi i z_{12} {\bf 1}_k \ .
\label{kcharge}
\end{equation}
This background breaks
the $U(\infty )$ symmetry down to an $U(k)$ symmetry. The fluctuations
$A_r,\phi_i$ are not block diagonal, which would correspond to fluctuations
within each brane, but also contain off diagonal components
corresponding to strings connecting distinct membranes,
thereby accounting for the full $kN\times kN$ matrix structure.
The matrices can be represented as a sum of tensor
products of $N \times N$ matrices and generators
of the $U(k)$ Lie algebra \cite{BSS,SJR}.
The $N \times N$ parts, in the $N \rightarrow \infty$ limit, are replaced by functions
on the membrane - thus (17), (18)
are now replaced by
\begin{eqnarray}
A_0 &\leftrightarrow & A^0_0(x_1,x_2)\  {\bf 1}_k + A^a_0(x_1,x_2)\  T^a  \\
A_r &\leftrightarrow & 2\pi z_{12} \ (A^0_r(x_1,x_2)\ {\bf 1}_k
                                + A^a_r(x_1,x_2) \ T^a ) \nonumber \\
\phi_i &\leftrightarrow & \phi^0_i(x_1,x_2)\ {\bf 1}_k + \phi^a_i(x_1,x_2)\ T^a
    \nonumber \ .
\label{othersk}
\end{eqnarray}
where $T^a$ are the traceless generators of the $SU(k)$ Lie algebra.
Commutators thus become commutators of fields in the adjoint
representation of $U(k)$, {\em e.g.} (\ref{commutator}) becomes
$$
     [\phi_i(x_1,x_2) ,\phi_j(x_1,x_2) ]_k
$$
and the $SU(k)$ part will survive.

The trace over $kN\times kN$ matrices is now represented as follows
\begin{equation}
 {\rm Tr} \leftrightarrow \sigma_0 \int \ dx_1dx_2 {\rm Tr}_k \ ,
\label{tracek}
\end{equation}
where ${\rm Tr}_k$ is the trace over the $k\times k$ structure. Note that
the total membrane charge of the multimembrane configuration is
\begin{eqnarray}
   Z_{12} = -\frac{i}{2\pi}
   \ Tr[X_1,X_2] &\leftrightarrow & \sigma_0 \int dx_1dx_2 z_{12} {\rm Tr}_k {\bf 1}_k
    \\ \nonumber
               &=& k \cdot {\rm (charge\ of\ a\ single\ membrane)}
\end{eqnarray}
as it should be. Plugging everything into the Lagrangian (\ref{basicL}),
we obtain
\begin{equation}
    {\cal L}_B \leftrightarrow
    \sigma_0 \int \ d^2 x  \ \frac{T_0}{2} {\rm Tr}_k \ \{ -\frac{1}{2}
       (F_{\mu \nu} F^{\hat{\mu} \hat{\nu}}) + D_{\mu} \phi_i D^{\hat{\mu}} \phi_i
     + \frac{1}{2} ([\phi_i ,\phi_j ]_k)^2
     - 2(2\pi z_{12} )^3 F_{12}
     - (2\pi z_{12} )^2 \ {\bf 1}_k \ \}
\label{U(k)L}
\end{equation}
where
$$
\begin{array}{rcl}
 F_{0r} & = & \partial_0 A_r(x) - \partial_r A_0(x) -i[A_0(x),A_r(x)]_k \\
 F_{12} & = & \partial_1 A_2(x) - \partial_2 A_1(x) -i[A_1(x),A_2(x)]_k \\
D_0\phi_i & = & \partial_0 \phi_i(x) -i[A_0(x),\phi_i(x)]_k \\
D_r\phi_i & =  & \partial_r \phi_i (x) -i[A_r(x),\phi_i(x)]_k
\end{array}
$$
We can also check the gauge transformation properties directly.
The Matrix Lagrangian (\ref{basicL}) is invariant under the $U(kN)$ gauge
transformations
\begin{eqnarray}
   \delta A_r &=& -i[U_r,\lambda ] + i [\lambda, A_r ] \\
   \delta \phi_i &=& i[\lambda , \phi_i ] \nonumber \\
   \delta A_0 &=& \partial_0 \lambda + i[\lambda ,A_0] \nonumber
\end{eqnarray}
where the gauge transformation parameter $\lambda$ (and everything else)
is a $kN\times kN$ matrix. In the $N \rightarrow \infty$ limit these become
\begin{eqnarray}
   \delta A_r(x) &\leftrightarrow & \partial_r\lambda (x) + i [\lambda (x), A_r(x) ]_k \\
  \delta \phi_i(x) &\leftrightarrow & i[\lambda (x) , \phi_i (x)]_k \nonumber \\
\delta A_0(x) &\leftrightarrow & \partial_0 \lambda (x) +i[\lambda (x),A_0(x)]_k \nonumber
\end{eqnarray}
and give the correct $U(k)$ gauge symmetry of (\ref{U(k)L}).

\bigskip

\subsection{Wrapped membrane backgrounds (p=2)}

\bigskip

We now compactify the Matrix theory on a two dimensional torus
$T^2$ in the $X_1,X_2$ directions.
This corresponds to compactifying M theory on $T^2 \times S^1$, since
one spatial
direction was already compactified.
We will then consider backgrounds of transverse membranes which wrap around
the torus $T^2$. As a result of the compactification, there
will be additional degrees of freedom in the theory, due to strings which
wind around the compact directions. As explained by
Taylor \cite{GRT}, they can be
accomodated in the Matrix theory by replacing each
partonic D0-brane by a countably infinite number of copies of it on the
noncompact covering space of the torus.
The vector space $V$,
on which the matrices act, then has a tensor product
structure
\begin{equation}
     V = V_N \otimes H^2 \ .
\label{space}
\end{equation}
The $N$-dimensional space $V_N$ is multiplied by a countably infinite
dimensional space $H^2$ associated with the countable infinity of copies
of D0-branes and strings stretching between them\footnote{Recently,
winding supermembranes in eleven dimensions were investigated in \cite{WPP}.}.

The description of the Matrix model becomes simpler upon performing
T-duality in directions $X_1,X_2$. The torus $T^2$ is replaced
by its dual torus $\hat{T}^2$, and the 0+1 dimensional quantum mechanics
becomes a 2+1 dimensional U(N) super-Yang-Mills
theory \cite{GRT,BFSS,Suss}.

Instead of analyzing the fluctuations of a wrapped transverse membrane
in the T-dual 2+1 dimensional Matrix theory, we will try
to recover a Lagrangian for the massless fluctuations directly from
the 0+1 dimensional theory on the initial torus $T^2$.
Our approach will be to construct a membrane on the covering space and  then
to demand periodicity of the spatial coordinates. We consider a constant
density $\sigma_0$ of D0-branes on the covering space. The total number
of D0-branes is thus infinite, consistent with a nonvanishing value
of the membrane charge, ${\rm Tr} [X_1,X_2] \neq 0$. The construction
then proceeds much as before: we represent the membrane background
$U_{1,2}$ as covariant derivatives with a U(1) magnetic field, acting
on functions of the membrane world volume,
\begin{eqnarray}
     U_1 &\leftrightarrow & 2\pi z_{12} (i\partial_1 + a_1)  \\
     U_2 &\leftrightarrow & 2\pi z_{12} (i\partial_2 + a_2) \nonumber
\end{eqnarray}
where ${\bf a} = (a_1,a_2) = -\frac{1}{2} f_{12} (x_2,-x_1) $ as before.
However, now the coordinates $x_1,x_2$ have a finite range:
\begin{equation}
    0 \leq x_r \leq  L_r \ \ , \ r=1,2
\end{equation}
where $L_1,L_2$ are the sizes of the torus $T^2$, and
we demand that all quantities are periodic up to gauge transformations.
With this range for the coordinates $x_1,x_2$, the membrane wraps once
around the torus. The trace is represented as in (\ref{trace1}), leading
to a finite value of total charge
\begin{equation}
   Z_{12} = -\frac{i}{2\pi} \ \sigma_0 \ \int \ d^2x \ [U^1,U^2]
          = \sigma_0 z_{12} L_1L_2 = \frac{L_1L_2}{(2\pi)^2} \ .
\label{2charge}
\end{equation}
for the wrapped membrane.

The fluctuation analysis proceeds as before, and leads to the same effective
2+1 dimensional Lagrangian (\ref{U(1)L}) as before.
The tension of the membrane can be checked
to be given by the relation (\ref{tension}), as it should.

Consider now 2 parallel membranes wrapped on $T^2$. In addition to
the excitations of open strings within each membrane, there are excitations
of strings which interpolate between the two membranes.
As discussed in \cite{HT}, these strings
do not have winding modes because they
are all homotopic to each other. Effectively, these strings behave as
if the spacetime would be non-periodic. However, the homotopy property
and the periodicity of the torus is seen in the possibility of introducing
Wilson lines which correspond to non-trivial gauge holonomy.
We will return to this issue shortly.

For two parallel membranes, we could write
\begin{eqnarray}
     U_1 &\leftrightarrow & 2\pi z_{12} \ (i\partial_1 + a_1) \otimes {\bf 1}_2 \\
     U_2 &\leftrightarrow & 2\pi z_{12} \ (i\partial_2 + a_2)
                                                  \otimes {\bf 1}_2 \nonumber
\label{twosimple}
\end{eqnarray}
as before, and then proceed exactly as we did in the previous section.
This leads to the 2+1 dimensional U(2) Yang-Mills Lagrangian (\ref{U(k)L}).
However, it should be possible to make distinction between two singly
wound (around $T^2$) membranes and a {\em single} membrane winding
twice around one of the cycles of $T^2$. This distinction can be made
as follows. We can add constant terms to (41) and define
\begin{eqnarray}
     U_1 &\leftrightarrow & 2\pi z_{12} \ [(i\partial_1 + a_1) \otimes {\bf 1}_2
     + \langle A_1 \rangle ] \\
     U_2 &\leftrightarrow & 2\pi z_{12} \ [(i\partial_2 + a_2) \otimes {\bf 1}_2
     + \langle A_2 \rangle ] \ . \nonumber
\end{eqnarray}
The constant terms $ \langle A_r\rangle ,\ r=1,2$ are U(2) Lie algebra valued. This
addition does not affect the total 2-brane charge $Z_{12}$, since
the commutator $[\langle A_1\rangle ,\langle A_2\rangle ]$ is
traceless under ${\rm Tr}_2$. However,
in order to leave the 2-brane charge {\em density} unaffected, we
must require that the $\langle A_1 \rangle $ and $\langle A_2\rangle $ commute.

Recall that the fluctuations $A_1,A_2$ around the background are
defined by
\begin{eqnarray}
     X_1 = U_1 +  A_1 &\leftrightarrow &
             2\pi z_{12} \ [(i\partial_1 + a_1) \otimes {\bf 1}_2
           + \langle A_1\rangle + A_1 ] \\
     X_2 = U_2 +A_2  &\leftrightarrow &
             2\pi z_{12} \ [(i\partial_2 + a_2) \otimes {\bf 1}_2
           + \langle A_2\rangle  + A_2 ]  \ . \nonumber
\end{eqnarray}
{}From these relations it is apparent that the constant terms $\langle A_r\rangle $
can be interpreted as constant backround values of the gauge fields $A_r$
in the U(2) Yang-Mills Lagrangian (\ref{U(k)L}). Thus, they can be
used \cite{HP} to induce gauge
holonomies ${\cal U}_r$, through the Wilson lines
$$
     {\cal U}_r = P\exp \{ i\oint_r \ A \}
$$
around the cycles of $T^2$. When the background values are both zero, the
holonomies are trivial,
$$
  {\cal U}_1 = {\cal U}_2 = {\bf 1}_2 \ ,
$$
around both cycles. From the IIA point of view, we then have a bound
state of two D2-branes (and D0-branes), both winding once around the
two cycles of $T^2$. But if we set
\begin{eqnarray}
     \langle A_1\rangle &=& \frac{\pi}{2L_1} \left( \begin{array}{cc} -1 & 1 \\
                1 & -1 \end{array} \right) \\ \nonumber
     \langle A_2\rangle &=& 0 \ ,
\end{eqnarray}
we get a non-trivial holonomy
$$
  {\cal U}_1 = \left( \begin{array}{cc} 0 & 1 \\ 1 & 0
                   \end{array} \right) \ .
$$
In this case,
the result is interpreted as a single D2-brane (with D0-branes) which
winds twice around the $X_1$ cycle of $T^2$.
Both cases yield the same 2-brane charge $Z_{12}$ which is twice the
charge (\ref{2charge}) of a single membrane. Generalizations to other
winding membranes can be obtained in similar manner.

\bigskip

\subsection{Longitudinal fivebrane backgrounds (p=4)}

\bigskip

The fivebrane of M theory admits a simple description in Matrix theory
only if it is wrapped around the longitudinal direction. Since the fivebrane
is boost invariant in its world volume directions, going to the infinite
momentum frame is more involved than for the transverse membrane.
Momentum is instead added by superimposing
a gravitational wave solution. However, in the case of a single fivebrane
such a configurations necessarily includes nonzero membrane charge as well.
To obtain a configuration with vanishing membrane charge one can take
two fivebrane solutions with mutually opposite membrane charges and then
combine them. In this section we will examine fluctuations around
both types of backgrounds. First, let us
summarize the backrounds and their properties:

\begin{description}

\item [(i)] an infinite longitudinal fivebrane with transverse membrane charge
density; this reduces in D=10 to a type IIA non-marginal bound
state $4+2\perp 2+0$

\item [(ii)] infinite longitudinal fivebranes
with transverse leftmoving
oscillations carrying momentum density in 11th direction; this reduces
in D=10 to a marginally bound $4 \parallel 0$  configuration

\end{description}

\noindent
In case (i), in the $N \rightarrow \infty$ limit the background is represented by
$$
 U_r \leftrightarrow \left\{ \begin{array}{l}
               2\pi z_{12} \ (i \partial_r + a_r )  \ \ \ r=1,2 \\
               2\pi z_{34} \ (i \partial_r + a_r )  \ \ \ r=3,4
             \end{array} \right.
$$
where $a_r$ is a U(1) background field with a field
strength $f_{rs} = \partial_r a_s - \partial_s a_r$,
with nonzero constant components $f_{12},f_{34}$ describing
magnetic flux densities in 1-2 and 3-4 planes,
$$
 f_{12} = \frac{1}{2\pi z_{12}} \ \ , \ \ f_{34} = \frac{1}{2\pi z_{34}} \ .
$$
A similar
analysis as in Section 2.1 yields an effective Lagrangian for the
bosonic fluctuations,
\begin{equation}
 {\cal L}_B = \sigma_0 \ \int \ d^4x \ \frac{T_0}{2} \{ -\frac{1}{2}
 (F_{\mu \nu} F^{\hat{\mu} \hat{\nu}}) + \partial_{\mu} \phi_i \partial^{\hat{\mu}} \phi_i
    - f_{rs} F^{\hat{r} \hat{s}}
    - \frac{1}{2} (f_{rs} f^{\hat{r} \hat{s}}) \}
\label{U(1)5L}
\end{equation}
where the indices are raised with the metric
\begin{equation}
    \hat{\eta}_{\mu \nu } = {\rm diag}
                         \ (1,-f^2_{12},-f^2_{12},-f^2_{34},-f^2_{34} ) \ ,
\end{equation}
and where $\sigma_0$ is the D0-brane density.

\noindent
In case (ii), the background is represented by covariant derivatives with
a selfdual U(2) background\footnote{For earlier studies of such
background configurations in non-abelian gauge
theories, see {\em e.g.} \cite{LVB}.} field:
\begin{equation} \begin{array}{ll} a_1 =0 & a_3 =0 \\
                a_2 = F_0 x_1 \sigma^3 & a_4 = F_0 x_3 \sigma^3 \ \ .
    \end{array}
\label{double5brane}
\end{equation}
The $\pm 1$ diagonal elements of $\sigma^3$ represent the superposition of
two solutions carrying opposite membrane charge. Note that the background
breaks the U(2) symmetry to U(1)$^2$.
The field strength $f_{pq}=\partial_p a_q - \partial_q a_p -i[a_p,a_q]$
satisfies the selfduality condition
\begin{equation}
  f_{pq} = \tilde{f}_{pq}  = \frac{1}{2} \epsilon_{pqrs} \ f_{rs} \ .
\end{equation}
The transverse volume of the fivebranes
becomes infinite in the $N \rightarrow \infty$ limit and
is given by $A=(2\pi )^4 Nz_{1234}$, where $z_{1234}$ is the longitudinal
fivebrane charge density. The D0-brane charge density $\sigma_0$ is
\begin{equation}
  \sigma_0 = \frac{N}{A} = \frac{1}{(2\pi )^4 z_{1234}} \ .
\end{equation}
It is related to the background field by
\begin{equation}
 2 \ \sigma_0 = \frac{1}{8\pi^2} {\rm Tr}_2 \ (f\wedge f) \ ,
\label{wedge1}
\end{equation}
which gives
\begin{equation}
            F_0 = \frac{1}{2\pi \sqrt{z_{1234}}} \ .
\end{equation}
Note that  $\sigma_0$ is the density of D0-branes per fivebrane; the total
density of D0-branes is  $2 \sigma_0$.

We then represent the background (ii) by the covariant derivatives
$$
 U_r \leftrightarrow 2\pi \sqrt{z_{1234}}
            \ (i\partial_r {\bf 1}_2 + a_r) \ \ \ r=1,2,3,4 \ .
$$
We can check that the
configuration carries a longitudinal 5-brane charge density
\begin{equation}
   -\frac{1}{8\pi^2} \epsilon_{pqrs}
                                      {\rm Tr} [U_pU_qU_rU_s] =  2\cdot z_{1234} \ ,
\label{5charge}
\end{equation}
where the prefactor 2 represents the presence of two fivebranes.
The fluctuations $A_0,A_r,\phi_i$ about the background are represented
by U(2) Lie algebra valued fields in 4+1 dimensions:
\begin{eqnarray}
    A_0 &\leftrightarrow & A^0_0(x)\  {\bf 1}_2 + A^a_0(x)\  T^a  \\
   A_r &\leftrightarrow & 2\pi \sqrt{z_{1234}}
          \ (A^0_r(x)\ {\bf 1}_2 + A^a_r(x) \ T^a) \nonumber \\
 \phi_i &\leftrightarrow & \phi^0_i(x)\ {\bf 1}_2 + \phi^a_i(x)\ T^a
     \ . \nonumber
\end{eqnarray}
where $T^a$ are SU(2) generators. The effective action
for the fluctuations is found to be
\begin{equation}
 {\cal L}_B = \sigma_0  \ \int \ d^4x \ \frac{T_0}{2} \ {\rm Tr}_2 \ \{
 - \frac{1}{2} (F_{\mu \nu} F^{\hat{\mu} \hat{\nu}})
    + D_{\mu} \phi_i D^{\hat{\mu}} \phi_i + \frac{1}{2} [\phi_i,\phi_j ]^2
 - f_{rs} F^{\hat{r} \hat{s}} - \frac{1}{2} (f_{rs} f^{\hat{r} \hat{s}}) \} \  \ ,
\label{U(2)5L}
\end{equation}
where the indices are raised with the metric
\begin{equation}
 \hat{\eta}_{\mu \nu } = {\rm diag } \ (1,-F^2_0,-F^2_0,-F^2_0,-F^2_0) \ .
\end{equation}
The energy density of the configuration is the sum of fivebrane plus
gravitational wave contributions $H= T+p_{11}$. The infinite momentum
frame Hamiltonian is found by subtracting $p_{11}$: $H_{\rm IMF} = T$.
T is found from the constant term in (\ref{U(2)5L}),
\begin{equation}
  T = 2 T_4 = 2 \frac{1}{(2\pi )^2} T_0 \ .
\end{equation}
This is as expected, since two longitudinal fivebranes are interpreted
as two D4-branes in the IIA theory.

\bigskip

\section{Scattering of branes}

Recently, there have been several studies of brane-brane scattering in
the context of Matrix theory \cite{AB,LM,L2,BC,L3,P,BB,CT1,CT2,PP}. These
calculations have demonstrated
agreement\footnote{Subtler issues and possible
discrepancies have also been discussed, see \cite{BL,GGR}.}
between 11 dimensional supergravity and Matrix theory
at one loop and even two loops \cite{BB}.
For Matrix theory compactified on torii, such
calculations amount to loop diagrams in Super-Yang-Mills theory
on the dual torus with magnetic backround fields encoding the brane
configuration and Higgs field VEVs specifying the kinematics of the
scattering problem. From the discussion in Section 2, it should be obvious
that a similar correspondence applies also for scattering
in uncompactified Matrix theory involving infinite branes.

Note that all the effective
actions (\ref{U(1)L},\ref{U(k)L},\ref{U(1)5L},\ref{U(2)5L}) can be
rewritten in a form
where the magnetic background fields are combined with the fluctuation
fields. Introducing a U(k) gauge field ${\cal A}_{\mu}$,
\begin{eqnarray}
  {\cal A}_0 &=& A_0 \\
  {\cal A}_r &=& a_r + A_r \nonumber
\label{fullfield}
\end{eqnarray}
and denoting its field strength by ${\cal F}_{\mu \nu}$, the
actions (\ref{U(1)L},\ref{U(k)L},\ref{U(1)5L},\ref{U(2)5L}) can
be written in the form
\begin{equation}
  {\cal L}_B = T_0 \sigma_0 \ \int \ d^px \ {\rm Tr}_k
\ \{ -\frac{1}{4} ({\cal F}_{\mu \nu } {\cal F}^{\hat{\mu} \hat{\nu}})
   + \frac{1}{2} ({\cal D}_{\mu} \phi_i {\cal D}^{\hat{\mu}} \phi_i )
  + \frac{1}{4} [\phi_i ,\phi_j ]^2 \}
\label{YMaction}
\end{equation}
where the covariant derivative ${\cal D}_{\mu}$ is taken with respect
to the field (57) which includes the background.
Now, after including fermions, gauge fixing and ghost terms,
we can compute scattering amplitudes from loop diagrams in the
appropriate background fields which encode the
information about the scattering objects and kinematical setup.

\subsection{D0 - D6+D0 Scattering}

We will perform a scattering calculation involving configurations
of D6-branes and D0-branes. Among various other configurations,
G. Lifschytz studied the scattering of 6+4+2+0 bound states from
D0-branes \cite{L2}. (Further discussion can be found in \cite{BL}.)
Recently, W. Taylor \cite{WT} showed
how to compose configurations of D6 branes
and D0-branes which do not carry D4 or D2 brane charges.
Such configurations\footnote{These
configurations are classically stable up to quadratic order.
They are thought to be related
to the supergravity black hole solutions of \cite{Shein} carrying
0-brane and 6-brane charges.} carry
a background U(4) gauge field
\begin{equation} \begin{array}{lll} a_1 =0 & a_3 =0 & a_5 =0 \\
                a_2 = F_0 x_1 \mu_1 & a_4 = F_0 x_3 \mu_2
                 & a_6 = F_0 x_5 \mu_3
    \end{array}
\end{equation}
with traceless U(4) matrices
\begin{eqnarray}
   \mu_1 &=& {\rm diag} (1,1,-1,-1) \\
   \mu_2 &=& {\rm diag} (1,-1,-1,1) \nonumber \\
   \mu_3 &=& {\rm diag} (1,-1,1,-1)  \ . \nonumber
\label{mus}
\end{eqnarray}
Analogously to (\ref{wedge1}), the above configuration gives a
D0-brane charge density
$$
   4\ \sigma_0 = \frac{1}{48\pi^3}
    {\rm Tr}_4 \ ( f \wedge f \wedge f) = 4\ \left( \frac{F_0}{2\pi } \right)^3 \ .
$$
As before, one can examine the fluctuations about this configuration
and obtain an effective U(4) action of the form (\ref{YMaction}) with $p=6$ and
a metric
$$
 \hat{\eta}_{\mu \nu } = {\rm diag} (1,-F^2_0,-F^2_0,
                                            -F^2_0,-F^2_0,-F^2_0,-F^2_0) \ .
$$
We have examined
the scattering of D0 particles from Taylor's D6+D0 brane configurations and
calculated the potential between  these objects.
The D6+D0 configuration can be understood in the same way as the
fivebrane with vanishing membrane charge of Section 2.3. It represents
a superposition of four 6+4+2+0 solutions which are chosen to give
vanishing D4-brane and D2-brane charges when combined.
The scattering calculation that follows reveals this structure, in
as much as the potential is found to be four times that between
a D0 particle and a 6+4+2+0 state.
In the Matrix theory 1-loop calculation
(which is the same as the 1-loop calculation in the effective
theory (\ref{YMaction}),
as we argued above), we encounter the following determinants
(the boson, ghost and fermion contributions in the background
gauge)
\begin{equation} \begin{array}{l}
 \det^{-3} \{ (-\partial^2_{\tau} + H +2c) \ {\bf 1}_4  \}
 \ \det^{-3} \{ (-\partial^2_{\tau} + H -2c) \ {\bf 1}_4  \} \\
 \det^{-2} \{  (-\partial^2_{\tau} + H ) \ {\bf 1}_4 \} \\
 \det \{  (-\partial^2_{\tau} + H +3c) \ {\bf 1}_4 \}
 \ \det^3 \{  (-\partial^2_{\tau} + H +c) \ {\bf 1}_4  \} \\
 \det^3 \{  (-\partial^2_{\tau} + H -c) \ {\bf 1}_4  \}
 \ \det \{ (-\partial^2_{\tau} + H -3c) \ {\bf 1}_4  \} \ \ ,
\end{array}
\end{equation}
where
$$
 H = r^2 + c (2(n_1+n_2+n_3)+3)  \ .
$$
Here $r$ is the distance between the D0-brane and
the 6+0 configuration, $c=1/F_0$,
and $n_1,n_2,n_3=0,1,\ldots$ . These determinants
are the same as those in the calculation by Lifschytz
of the D0 - 6+4+2+0 potential, except for additional
$4\times 4$ unit matrix factors. The unit matrices signal that the D0-brane
sees the four 6+4+2+0 sublayers in the 6+0 configuration, thus the
potential between the 6+0 configuration and the D0-brane will be four times
that obtained by Lifschytz \cite{L2}:
\begin{equation}
     V(r) = 4 \cdot \frac{3}{16} \frac{1}{F_0r} \ .
\label{potential}
\end{equation}

The corresponding supergravity result is easily obtained
by considering the 6+0 configuration as a probe moving
in the D0-brane background. The calculation  is performed in the
same manner as by Chepelev and Tseytlin \cite{CT1}, who considered
various configurations involving 4-branes and 5-branes. Their paper
also collects a number of useful formulae which we will draw from in
the following. The effective action for the 6+0 configuration is
given by\footnote{For the effective action we will use Tseytlin's
truncated version of the non-abelian Born-Infeld action \cite{NABI},
valid in cases,
such as the present one, where the worldvolume field strengths commute.}
\begin{equation}
 S_6 = \int \ d^7 \xi \ {\rm Tr} \{ -T_6 e^{-\phi } \ \sqrt{\det [g_{\mu \nu}
\frac{\partial X^{\mu}}{\partial \xi^i} \frac{\partial X^{\nu}}{\partial \xi^j}
 + F_{ij}]} + \mu_6 (C_0 F_{12}F_{34}F_{56} + \cdots ) \} \ ,
\end{equation}
where $\cdots$ indicates various Chern-Simons terms which are irrelevant
for our present purposes. In our units, we have $\mu_6 =T_6$. The field
strength in the worldvolume is
given by $F_{12}=F_0\mu_1,F_{34}=F_0\mu_2,F_{56}=F_0\mu_3$, with
$\mu_{1,2,3}$ defined in (60). The spacetime fields to be inserted
into $S_6$ are those induced by a D0-brane source ``smeared'' in directions
$x^1,\ldots ,x^6$:
\begin{eqnarray}
ds^2 &=& H^{-1/2}_0 dt^2 - H^{1/2}_0
      (dx^2_1 + \cdots +dx^2_9) \\ \nonumber
e^{-\phi} &=& H^{-3/4}_0 \ \ ; \ \ C_0~=~H^{-1}_0 -1 \\ \nonumber
H_0 &=& 1 + \frac{Q^{(6)}_0}{r} \ \ ; \ \
                     r^2~=~x^2_7 + x^2_8 + x^2_9 \\ \nonumber
Q^{(6)}_0 &=& \frac{g}{2} (2\pi )^{5/2} \ .
\end{eqnarray}
Substituting into $S_6$ yields
$$
  S_6 = -4T_6 \int \ d^7x \ \{ H^{-1}_0 (H_0 + F_0^2)^{3/2}
                     - (H^{-1}_0 -1)F_0^3 \} \ .
$$
To compare with the Matrix theory result we should
take $r,F_0 \rightarrow \infty $, corresponding to the large distance interaction
between objects in the infinite momentum frame of M theory. Then
$$
 S_6 \approx -4T_6 \int \ d^7x \ \{ \frac{3}{8} \frac{H_0}{F_0}
   + F_0^3 + \frac{3}{2} F_0 \} \ .
$$
Now we can read off the potential,
$$
  V(r) \approx 4 \cdot \frac{3}{8} \frac{T_6 Q^{(6)}}{F_0r}
   = 4\cdot \frac{3}{16} \frac{1}{F_0r} \ ,
$$
in agreement with the Matrix theory result (\ref{potential}).

\section{Conclusion}

We have seen that by taking the $N \rightarrow \infty$ limit of Matrix theory in a
particular way, it is possible to recover much of the known physics of
D-branes in IIA theory.  In particular, by representing the coordinate
matrices as covariant derivatives we arrived at the correct Yang-Mills
actions governing the low energy dynamics of D-branes.  As discussed, these
actions are properly interpreted as  Born-Infeld actions expanded around
large magnetic field backgrounds.  This interpretation was verified
explicitly, including checking numerical factors, in the case of a single
D2-brane.  We also used the effective actions to compute the potential
between a D0-brane and a configuration of D6-branes and D0-branes, and saw
that the result was in agreement with supergravity.

Finally, although in this paper attention has been restricted to
the $N \rightarrow \infty$ limit, it would be interesting to investigate D-brane actions at
finite N. Despite the absence of infinite BPS branes for such N, it is
 possible to compare various processes with the predictions of
supergravity compactified along a null direction \cite{Nfin,BBPT}.  To understand
such processes better, it would be useful see
 to how much of our techniques may be carried over to finite N.

\bigskip

{\Large {\bf Acknowledgements}}

\bigskip

We would especially like to thank Soo-Jong Rey for discussions which
motivated this investigation. We also thank A.~Tseytlin
for remarks on Matrix theory scattering calculations.
E.~K-V. would
like to thank the Helsinki Institute of Physics for hospitality
during the writing of this work.

\bigskip

redpajama_set_name: RedPajamaArXiv


text:
You are here: Home / Soup Du Jour / OneJax Institute Hosts 100th Annual Interfaith Thanksgiving Gratitude Service
OneJax Institute Hosts 100th Annual Interfaith Thanksgiving Gratitude Service
The OneJax Institute at the University of North Florida will celebrate its 100th annual Interfaith Thanksgiving Gratitude Service at 6 p.m. Thursday, Nov. 16, at Congregation Ahavath Chesed—The Temple, located at 8727 San Jose Blvd. A fellowship reception will follow at 7 p.m.
This annual service has taken place in Jacksonville since 1918 and pays homage to the sacred passages, prayers, songs and traditions that exalt the quality of gratitude for the community's blessings.
"This is a remarkable milestone. One hundred years ago, Rabbi Israel Kaplan at the Temple on Laura and Ashley Streets, invited Rev. Walter Pierce at the Unitarian Church to join in a 'Union Service' on Thanksgiving Day," said Nancy Broner, OneJax executive director. "Over the years, additional faiths joined in to offer thanks and gratitude for all we appreciate as a community. We look forward to celebrating with the entire community."
The theme of this year's special service is "Reasons for Hope" and will include a procession of faith leaders and clergy. Expressions of gratitude from each tradition will follow and will include representatives from the Baha'i, Buddhist, Christian, Hindu, Jewish, Muslim, Sikh and Native American faiths, among others. An interfaith choir will also participate. This year, more than a dozen faiths and traditions will be represented.
"If ever there was a need to be reminded that we aren't alone and that, despite our differences, we share many of the same values and beliefs, it's right now," said Broner. "Our world is divided, we've endured and observed natural disasters and have witnessed unexplainable acts against innocent victims. In the midst of all this, the interfaith service reminds us to treat one another with kindness, to be grateful for all that we have and to approach each other with compassion."
The service is free and open to the public. Participants are encouraged to bring canned and dry goods, which will be donated to Feed a Needy Neighbor. RSVPs are appreciated at https://tinyurl.com/100gratitude or call 904.620.1529.
Since 2012, OneJax has been an Institute at the University of North Florida. Through education, community building and advocacy, OneJax Institute works to make Northeast Florida a better place for everyone by celebrating differences and identifying all we have in common. Its core programs include Metrotown, an intensive, week-long teen diversity program; LOUD (Leaders of United Diversity), where Metrotown graduates bring the message of respect and appreciation for religious, racial and cultural differences into their schools; Interfaith and Community Forums, periodic forums for public dialogue on diversity and community building; and Advocacy, working to promote issues of importance to the OneJax mission.
In addition, OneJax partners with the UNF College of Education and Human Services on Project Breakthrough, an initiative to change the story of race in Jacksonville. The organization also partners with The Florida Times-Union, WJCT Public Broadcasting and the Jacksonville Human Rights Commission on Civil Discourse Forums, promoting civil conversations around difficult or uncomfortable topics and issues. For more information go to www.onejax.org or call 904.620.1529.
Filed Under: Soup Du Jour Tagged With: OneJax Institute, university of north florida

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text:
ANGA COM preview event highlights importance of IP
16th February 2015 @ 12:01
The growing importance of IP as a complement to cable distribution was the key highlight of German trade show ANGA COM's preview event last week.
Jürgen Magull of M7 Deutschland, which last year acquired the Eutelsat-owned Kabelkiosk platform, opened the event with an overview on the development of TV usage, using market data to show that TV usage via tablets and smartphones has gained in importance. He told attendees that IPTV was not only an alternative as first screen offering, but also complemented DVB-C to serve the second screen devices.
Daniel Hesselbarth of Liberty Global-owned Unitymedia KabelBW, presented the latest version of the Horizon platform which includes DVB-C as well as IP services, while Gernot Jaeger of Zattoo highlighted the OTT providers strategy of providing third party operators with white label offerings for the TV and as a second screen complement to established television offerings.
Other presentations included that of Heiner Meyer of alternative carrier EWE TEL, who highlighted the company's delivery of television using traditional cable technology (LWL TV) via fibre networks and IPTV via DSL connections. DSL customers can choose between online TV via PC and the TV App for tablets and smartphones.
"IPTV is rapidly gaining importance for TV provisioning. This was also reflected by the great interest in the ANGA COM workshop. When introducing IPTV in addition to existing DVB-C services the consumer's Quality of Experience may not be compromised," said Carsten Engelke, of ANGA.
"Before launching concepts with unicast and multi-cast solutions these have to be thoroughly examined to ensure the economic success of the service implementation. The trend towards All-IP with DOCSIS 3.1 is advancing. Cable networks are ideally positioned for this."
The ANGA COM exhibition and congress will take place from 9 to 11 June 2015 in Cologne, Germany.
Tags: ANGA COM, Germany
Four agencies in for UEFA marketing rights
Four sports marketing agencies have reportedly emerged as the leading bidders in UEFA's club competitions rights distribution auction. According to SportBusiness, UEFA's long-time agency partner Team Marketing – which has distributed the rights since 1992 – has submitted a bid, while other large agencies are also bidders including IMG, Infront and Relevant Sports Group. All […]
Starlink sets out stall for India
SpaceX-owned Starlink has said that it will apply for a commercial licence in India in 2022. Expansion into India would see the company provide broadband and other services in the country. The news comes via Sanjay Bhargava, Starlink Country Director, India at SpaceX, who posted an update on LinkedIn stating: "We hope to have applied […]
Discovery emerges as potential BT Sport suitor
Discovery has reportedly entered into talks with BT to buy BT Sport. This is a late development for the for-sale broadcaster, which is said to be in the late stages of negotiations with DAZN regarding a £600 million takeover deal. By contrast to DAZN, which reportedly wants to buy the broadcaster, the FT claims that […]
New board for Open Fiber following takeover
Italian broadband operator Open Fiber has announced the appointment of Mario Rossetti as its new CEO. The announcement comes less than a month after Australian investment bank Macquarie and state lender Cassa Depositi e Prestiti (CDP) won EU regulatory approval to takeover the operator. In addition to the appointment of Rossetti – who replaces interim […]
Vevo Pop channel launches on rlaxx TV
Addressable advertising in France ramps up with Bouygues launch
Digital UK and Freesat come together
Pluto TV taps Blue Ant for 650 hours of content
ICYMI: @Microsoft to buy Call of Duty publisher Activision Blizzard in US$70 billion deal digitaltveurope.com/2022/01/19/mic… https://t.co/hloJWZUCzT


"Fake news" is not a term that many of us were familiar with this time last year, but now the term is being bandied around on a daily basis thanks to its usage by President Donald Trump.
However, this is not just a political phenomenon. Businesses are having to quickly wake up to the potential impact that "fake news" can have on them, with campaigns launched to boycott and manipulate public perceptions of brands. Furthermore, what happens if a senior individual in a company becomes a victim of fake news - which can in turn impact the company's reputation.
Companies also need to be careful not to inadvertently share "fake news" - dragging themselves into a scandal. Employees must be vigilant about the content they share online.
But surely people can tell the difference between what is real and what is fake? Well apparently not!
Stanford's Graduate School of Education carried out a study on this - assessing more than 7,800 school and college students across the United States on their ability to assess information sources. The results are rather shocking.
It's not that people who believe "fake news" are "dim" but that the "fake news" replicates the formats of trusted news sources so well that it is extremely difficult to tell fact from fiction.
The severity of the impact of "fake news" is reflected by Brussels' decision to crack down on social media companies who have been accused of spreading such content.
Whilst once considered to be a funny "Trumpism" "fake news" should not be taken lightly by companies - the European Commission most certainly isn't.


Catch up on all the latest news, gossip and info about Caroline Manzo and The Real Housewives of New Jersey. Read our blog to keep in touch with all the juicy scoop.
Is Chris Manzo Moving Out Of New Jersey?
The Brownstone which has been featured on the Real Housewives of New Jersey that is owned by Caroline Manzo's husband Albert, is in financial trouble, according to a new report. A New Jersey state judiciary clerk confirmed that Albert owes $208,012.77 in state taxes from 2015. The Brownstone House Inc.
Would Caroline Manzo Return to RHONJ?


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Did you know that Halloween is celebrated in France too?
Did you know that we have a French beautician in Bristol?
L'Ecole normande ou l'Ecole Normale?
L'Ecole normande ou l'Ecole Normale?
Another Nuit Blanche in Paris last night!


text:
The science of cloud seeding
ACS News Service Weekly PressPac: June 01, 2016
"Firm footing for cloud seeding"
Chemical & Engineering News
Experiments to seed clouds and coax them to produce more rain started 70 years ago. Early practitioners claimed a 10 percent boost in precipitation, but their studies lacked statistical rigor. The science of rainmaking has evolved since then — but how reliable is it now? An article in Chemical & Engineering News (C&EN), the weekly newsmagazine of the American Chemical Society, takes a look.
Janet Pelley, a contributing editor at C&EN, reports that for cloud seeding science to come into its own, it needs to address some major challenges. To start, scientists have yet to understand a critical step in natural rainmaking: ice nucleation. This process involves water vapor freezing onto particles, which leads to precipitation. Another significant glitch in experimenting with seeding is the difficulty with running controlled experiments in real clouds. Once a cloud is treated, scientists can't measure how much rain it would have produced if left alone.
To chip away at these obstacles, scientists have developed more sophisticated experiments and simulations using sensing tools and computer models. Recent multi-year studies have found hints that seeding might yield a boost in precipitation. But results weren't statistically significant. Remote sensing is giving scientists a better view into cloud dynamics in real time and could help advance the science. As dozens of countries invest millions of U.S. dollars in cloud seeding, the new studies could be well worth the effort.
Whether seeding clouds succeeds in boosting rainfall remains up in the air.
Credit: Jim Brandenburg/Minden Pictures/Newscom


An entrepreneur with over 15 years of hands-on experience and proven business and design results. Always seeking new ways to maximize the WOW effect of products, crafting each component with the care and attention to detail that creates complete, end-to-end solutions.
My extensive experience in business development, product management, e-branding and interaction design enables me to provide a multi-faceted and multi-disciplinary approach. I specialize in inclusive design and see myself as a web accessibility evangelist.
Over 15 years of hands-on experience in product design, e-branding, e-Learning and interaction design.
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Already from the very beginning she had become from just a User Interface designer to the single person we turned to when we had to think about the concept of the interface and functionality so it would be perfect for the users.
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The New Yorker has published the first serial excerpt of St. Marks Is Dead.
"You grew up on St. Marks Place?" people sometimes ask me, as if they didn't know children could. Or, "You grew up on St. Marks Place?" implying that I seem too normal to come from a place known for Mohawks and tattoo parlors. Then, invariably, these strangers pity me for having missed the street's golden era. St. Marks bohemians—those who were Beats in the fifties, hippies in the sixties, punks in the seventies, or anarchists in the eighties—often say that the East Village is dead now, with only the time of death a matter of debate. New Yorkers are street-proud, and every neighborhood invites its share of good-old-days lamenting. But just as St. Marks Place has long been an amplified corner of the city—louder, drunker, more garish than its neighbors—today it seems to evoke a more intense nostalgia.


text:
Newbridge kan syfta på följande platser:

Irland

 Avoca (ort i Irland), Leinster, Wicklow,
 Droichead Nua, ort, Leinster, Kildare,

Storbritannien

 Newbridge, Edinburgh, Skottland,
 Newbridge, Caerphilly, ort i Wales,
 Newbridge, Dumfries and Galloway – en ort i Dumfries and Galloway, Skottland
 Newbridge, East Sussex – en ort i East Sussex, England
 Newbridge, Hampshire – en ort i Hampshire, England
 Newbridge, Isle of Wight – en ort i Isle of Wight, England
 Newbridge, Kenwyn – en ort i Kenwyn, Cornwall, England
 Newbridge, Lancashire – en ort i Lancashire, England
 Newbridge, North Yorkshire – en ort i North Yorkshire, England
 Newbridge, Oxfordshire – en ort i Oxfordshire, England
 Newbridge, Sancreed – en ort i Sancreed, Cornwall, England
 Newbridge, Shropshire – en ort i Shropshire (distrikt), Shropshire, England
 Newbridge, Somerset – en ort i Bath and North East Somerset, Somerset, England
 Newbridge, West Midlands – en ort i Wolverhampton, West Midlands, England
 Newbridge, Wrexham – en ort i Wrexham, Wales
 Newbridge on Usk – en ort i Monmouthshire, Wales
 Newbridge-on-Wye – en ort i Powys, Wales

Robotskapade Irlandförgreningar
Robotskapade Storbritannienförgreningar

redpajama_set_name: RedPajamaWikipedia


text:
Surgical Sealants and Adhesives Market Global Overview 2019, Development Pipeline, Industry Analysis, Size, Share, Business Growth Opportunities, Top Company Profile, Regional Forecast to 2023
Market Research Future Releases
An expert on premium research reports, Market Research Future has added a report titled "Global Surgical Sealants and Adhesives Market 2023" to its offering. Global Surgical Sealants and Adhesives Market is expected to grow significantly over the forecast period. It is anticipated that the market held a market value of USD 2.12 billion in 2017 and is projected to grow at a CAGR of 9.3% over the forecast period.
Bard, Inc. (US), Johnson & Johnson (UK), Baxter International, Inc. (US), Medtronic plc (US), B. Braun Melsungen AG (Germany), Cohera Medical, Inc. (US), Sanofi Group (France), Sealantis, Ltd (Israel), Vivostat A/S (Denmark), and Ocular Therapuetix, Inc. (US) are some of the key players in the global surgical sealants and adhesives market.
Get Free Sample Copy @ https://www.marketresearchfuture.com/sample_request/7005
Growing prevalence and incidence of various disorders, growth in the number of accidents, and growth in the number of surgeries are expected to drive the growth of market. According to the Centers for Disease Control and Prevention (CDC), each year around 630,000 Americans die from heart disease. On other hand, lack of reimbursements policy; and extensive clinical data requirements for launching products can restrain the market growth over the assessment period.
Geographically, the Americas is expected to dominate the global surgical sealants and adhesives market owing to the presence of well-developed healthcare sector, growing prevalence and incidence of various disorders, growth in the number of accidents, and growth in the number of surgeries. Europe is expected to hold the second largest position in the global surgical sealants and adhesives market owing to the growing prevalence of chronic diseases coupled with increasing adoption of new technologies. Asia-Pacific is expected to be the fastest growing market owing to the large population base of the diabetic patients and increasing developments in healthcare segment. Furthermore, the Middle East and Africa region is expected to account for the least market share in the global surgical sealants and adhesives market.
The global surgical sealants and adhesives market has been segmented into product, indication, application, and end user.
Based on product, has been segmented into natural/biological sealants and adhesives and synthetic and semisynthetic sealants and adhesives. The natural/biological sealants and adhesives and synthetic segment is accounted for the largest share segment of the market in 2017.
The market, by indication, has been segmented into surgical hemostasis, tissue sealing, and tissue engineering.
The market, by application, has been segmented into general surgeries, cardiovascular surgeries, central nervous system surgeries, orthopedic surgeries, urological surgeries, and others.
Browse Premium Research Report Enabled with Respective Tables and Figures @ https://www.marketresearchfuture.com/reports/surgical-sealants-and-adhesives-market-7005
Detailed Table of Contents for Surgical Sealants and Adhesives Market
Table 1. Global Surgical Sealants And Adhesives Market Synopsis, 2018–2023
Table 2. Global Surgical Sealants And Adhesives Market Estimates And Forecast, 2018–2023 (USD Million)
Table 3. Global Surgical Sealants And Adhesives Market, By Region, 2018–2023 (USD Million)
Table 4. Global Surgical Sealants And Adhesives Market, By Product, 2018–2023 (USD Million)
Table 5. Global Surgical Sealants And Adhesives Market, By Indication, 2018–2023 (USD Million)
Table 6. Global Surgical Sealants And Adhesives Market, By Application, 2018–2023 (USD Million)
Table 7. North America: Surgical Sealants And Adhesives Market, By Product, 2018–2023 (USD Million)
Table 8. North America: Surgical Sealants And Adhesives Market, By Indication, 2018–2023 (USD Million)
Table 9. North America: Surgical Sealants And Adhesives Market, By Application, 2018–2023 (USD Million)
Table 10. US: Surgical Sealants And Adhesives Market, By Product, 2018–2023 (USD Million)
Table 11. US: Surgical Sealants And Adhesives Market, By Indication, 2018–2023 (USD Million)
Table 12. US: Surgical Sealants And Adhesives Market, By Application, 2018–2023 (USD Million)
Table 13. Canada: Surgical Sealants And Adhesives Market, By Product, 2018–2023 (USD Million)
Table 14. Canada: Surgical Sealants And Adhesives Market, By Indication, 2018–2023 (USD Million)
Table 15. Canada: Surgical Sealants And Adhesives Market, By Application, 2018–2023 (USD Million)
Table 16. South America: Surgical Sealants And Adhesives Market, By Product, 2018–2023 (USD Million)
Table 17. South America: Surgical Sealants And Adhesives Market, By Indication, 2018–2023 (USD Million)
Table 18. South America: Surgical Sealants And Adhesives Market, By Application, 2018–2023 (USD Million)
Table 19. Europe: Surgical Sealants And Adhesives Market, By Product, 2018–2023 (USD Million)
Figure 1. Research Process
Figure 2. Segmentation For Global Surgical Sealants And Adhesives Market
Figure 3. Segmentation Market Dynamics For Global Surgical Sealants And Adhesives Market
Figure 4. Global Surgical Sealants And Adhesives Market Share, By Product, 2017
Figure 5. Global Surgical Sealants And Adhesives Market Share, By Indication, 2017
Figure 6. Global Surgical Sealants And Adhesives Market Share, By Application, 2017
Figure 7. Global Surgical Sealants And Adhesives Market Share, By Region, 2017
Figure 8. North America: Surgical Sealants And Adhesives Market Share, By Country, 2017
Figure 9. Europe: Surgical Sealants And Adhesives Market Share, By Country, 2017
Figure 10. Asia-Pacific: Surgical Sealants And Adhesives Market Share, By Country, 2017
Figure 11. Middle East & Africa: Surgical Sealants And Adhesives Market Share, By Country, 2017
Figure 12. Global Surgical Sealants And Adhesives Market: Company Share Analysis, 2017 (%)
Figure 13. C. R. Bard, Inc.: Key Financials
Figure 14. C. R. Bard, Inc.: Segmental Revenue
Figure 15. C. R. Bard, Inc.: Geographical Revenue
Figure 16. Johnson & Johnson: Key Financials
…TOC Continued!
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The NCAA basketball tournament is not providing much madness. It's pure chalk.
Perhaps this week's WGC-Dell Tech Match Play will make up for the lack of upsets in this year's NCAA Tournament.
The current WGC-Match Play format allows for round-robin play over the first three days (starting on Wednesday) and then single elimination for the 16 golfers that escape from the group stage.
There are pros and cons to this format but it does allow every golfer at least two meaningful matches (possibly one meaningless match). The previous format of one-and-done would only guarantee one match that mattered. If you lost your opening match you were done. Now you can overcome one bad day and hope the rest of your group beats up on each other.
Dave Tindall already broke down the format and course which is Austin Country Club for the fourth straight year. Check out his Euro-Based Match Play Preview. To read more about the course and past quotes from the golfers, head over to the Fantasy Golfanac.
Trying to keep narratives out of the equation, here is how I will break down each group. I will look at three different angles (long-term play, current form, and match play history). I will state the two top golfers based on each model and then piece together my final verdict for each group.
Long-term Performance: Weighted Stroke Play Performance on the PGA TOUR and Euro Tour over the last year.
Current Form: Weighted Performance over the Last 12 weeks on the PGA TOUR and Euro Tour.
Match Play History: Hole-by-Hole performance over Average in all singles matches over the last 10 years. This also accounts for opponent strength.
Final Verdict: On paper this looks like a two-horse race but stranger things have happened. DJ won this event just two years ago but last year he got bounced in Group Stage with an 0-3-0 record.
Final Verdict: Woodland went 0-for-2 at Dove Mountain but he was 6-1-0 at TPC Harding Park and currenly holds a 2-1-1 record at Austin CC. Not too shabby for a singles resume. As for the favorite, Rose, he went 1-1-1 during his 2016 debut at Austin Country Club and this will be his first time returning to the course.
Final Verdict: Koepka has been very spotty in 2019, outside of his runner-up finish at the Honda. On the bright side, he holds a 9-5-1 record in match play while doing it against some strong opponents. Noren is the Match Play darling but his form is way too far off the radar, this time around.
Final Verdict: Harding has been sneaking under the radar overseas, including a win and runner-up finish in his last two starts. McIlroy has been drawing all the spotlights and for good reason. He hasn't finished worse than T6 in his last six starts and he capped off that run with a win at THE PLAYERS. Will that take away some of the hunger or will he look to add another Match Play trophy to his case? He won the 2015 edition at Harding Park.
Final Verdict: Bjerregaard has a 1-3-0 record at the Paul Lawrie Match Play but he's a much-improved golfer over the last year. Wallace is just 0-1 at the PL Match Play so it's not enough to build a case for or against. His current form does make him the mostly likely knock JT over his throne.
Final Verdict: Bryson took Noren down to the wire at the Ryder Cup which actually a positive outcome, given the strong record of Noren in singles. Barnrat has a much larger sample size of match play success if you want to take that angle. He went 3-0 here last year in group play to escape from Rahm's group.
Final Verdict: Molinari may be a popular pick this week, thanks to his Ryder Cup performance. We need to remember that most of that was done alongside Tommy Fleetwood. His overall singles record is nothing to write home about. He is 2-3-0 here at Austin CC.
Final Verdict: A tough draw for Rahm who runs into some Pete Dye specialists in Matt Kuchar and Si Woo Kim. Kooch has won 60% of his singles matches over the last 10 years which is 12th best in the field of all golfers with 20+ matches played over that time.
Final Verdict: Going back to that same stat of win percentage over the last 10 years, RCB ranks 5th in this week's field (of golfers with 20+ matches played). He is 7-4-1 at Austin Country Club.
Final Verdict: Casey just won at the Valspar but he got edged slightly in the form department, thanks to an implosion at THE PLAYERS. The Englishman is 5-3-1 at Austin Country Club. Will it be an easy road? Maybe not since CH3 went 3-0-0 during group play last year before losing to Kiradech Aphibarnrat in the Round of 16.
Final Verdict: It looks like a lot of possible outcomes based on the lists above. All four of the golfers show up in the top two in at least one angle. Stanley got through group play last year while Oosthuizen was the runner-up finisher here in 2016.
Final Verdict: Stenson is making his debut at Austin Country Club. He's won his last three worldwide singles matches but in the long-term, his resume is very pedestrian. Jason Day is the man to beat here as long as his body holds up for the week. That is always a question mark but it passed the test in 2016 when he tore through the tournament and beat Louis Oosthuizen in the title match.
Final Verdict: The last five appearances at this event has yielded a 2-4-0 record for Tiger Woods. That was at Dove Mountain so maybe the new course will get him back on track. Other than his loss to Jon Rahm at the 2018 Ryder Cup, he is 4-0-1 in Ryder Cup and Presidents Cup matches over the last 10 years. This looks like a two-horse race between Tiger and Cantlay.
Final Verdict: Kisner made it to the finals here last year so don't count him out. However, the baseline stats from Finau and Poulter are in a tier above Kis and Keith Mitchell.
Final Verdict: It's still weird to see Spieth's baseline numbers stoop so low. The big numbers have been his downfall recently so perhaps the match play format will be to his liking. A return to a familiar venue certainly can't hurt, either. However, he has to deal with the defending champ in his group and also Billy Horschel who looks like a lively sleeper as the 38 seed.
Final Verdict: It looks like it will be a battle of the last two Masters champs. Reed was really struggling with his game last week but he's always one of the toughest outs in the head-to-head format. He's won more than 60% of his singles matches over the last 10 years but Garcia's singles record over the time is very similar but he also has current form in his favor.
Hopefully, this quick rundown has given you some info to snack on. Keep an eye out for the Expert Picks which will include our predicted picks for the event.
Update: I've included the Top 15 performers via each angle.


The Reflexology Association of Australia is excited to invite all members and other interested parties to the 2020 Conference 'Vision to the Future' being held on 16th to 18th October 2020 at the Novotel, Darling Harbour, Sydney NSW. Come celebrate our Vision to the Future' Conference and immerse yourselves in this educational and entertaining event.
To strenghten reflexology and the knowledge of reflexologists through evidence-based practice, research, and promotion.


PASADENA - Brittany Percin and Alex Janosi have been named CSCAA Scholar All-America and Honorable Mentioned, respectively.
The Caltech men's and women's swimming & diving teams added another pair of accolades to a stellar 2018, with both teams earning Scholar All-America distinction according to an annual release from the College Swimming Coaches Association of America.
Junior swimmer Brittany Percin made a successful debut in the NCAA Division III Swimming & Diving Championships this week, competing in three events and scoring as the SCIAC's top finisher in two out of the three events.
The 2018 Caltech men's and women's swimming & diving teams will have not one, but two Beavers represent the program at the 2018 NCAA Division III National Championships.
Junior swimmers Brittany Percin and Gemma Takahashi have earned all-SCIAC recognition for their efforts at the 2018 SCIAC Championships last week.
Junior Brittany Percin got back to the podium on the final day of the women's swim & dive SCIAC Championships on Saturday when she claimed a second-place finish in the 200 Fly finals.
Junior Gemma Takahashi of Caltech women's swim & dive became a SCIAC champion for the first time ever on Friday when she edged out a field of eight other swimmers in the 100 Butterfly at the SCIAC Championship meet.
The Caltech women's swimming & diving team scored meaningful points in both swimming and diving competitions at the 2018 SCIAC Championships to move up one spot following Friday's events.
Junior Brittany Percin played a major role in the Caltech women's swim & dive team breaking four records at the SCIAC Championhips on Wednesday's opening day.
Head Coach Paul Hughes and the Caltech men's and women's swim & dive teams head to Commerce for this weekend's SCIAC Championships looking to improve on last season's fifth- and ninth-place finishes.
Caltech women's swimming & diving closed out the regular season with another series of strong performances against Chapman University on Saturday morning ahead of next week's SCIAC Championships.
Freshman diver Krystin Brown picked up her first second-place diving finish in a double-dual meet against Pomona-Pitzer Colleges and California Lutheran University on Saturday morning.
The Caltech men's and women's swim & dive teams have been recognized as College Swimming & Diving Coaches Association of America Scholar All-America Teams for a second consecutive year under Head Coach Paul Hughes.
Freshman swimmer Jessica Sun added another Caltech breast stroke record to her fantastic rookie season at Saturday's Claremont-Mudd-Scripps-hosted double-dual meet with CMS and Occidental College.
Freshman Jessica Sun of the Caltech women's swimming & diving team broke the record for the women's 400-yard individual medley and lifted her team to a 125-100 victory over Mills College on Sunday afternoon.
Caltech women's swim & dive opened the new year with another program record against Whittier College on Saturday after a two-month break from competition.
Sophomore Brittany Percin and freshman Jessica Sun combined to break three of their old records in Saturday's SCIAC dual meet at the University of La Verne.
Freshman swimmer Jessica Sun is the seventh Caltech scholar-athlete to be featured in the new episodic web series, Beaver of the Week.
Rookie Jessica Sun broke a pair of records in her collegiate debut as the Caltech women's swim & dive team opened the 2017-18 season against the University of Redlands on Saturday.
A wildly successful first season under Head Coach Paul Hughes has generated some buzz around the Caltech men's and women's swimming & diving teams heading into the 2017-18 season.
The Caltech swimming & diving teams have added six men and two women first-years to fill key roles for the 2017-18 season.
Caltech swimming & diving has released its 2017-18 schedule; the season is set to open at home with a SCIAC dual meet against the University of Redlands on Saturday, Nov. 11 at 10:30 a.m.


text:
The Episcopal Church, Transfigured
I'm almost at a loss for words.
Yesterday the House of Deputies—one of the two Houses in The Episcopal Church's bicameral system of governance – passed resolutions D019 and D002. The House of Bishops had done the same on Saturday afternoon. Both resolutions add "gender identity and expression" to the Church's nondiscrimination canons. D019 addresses access of lay people to the life and governance of the church – so, for instance, it clarifies that transgender people can be Eucharistic ministers, vestry members, retreat attendees or leaders, etc. D002 affirms that transgender people can be ordained leaders. These resolutions addressed an already/not yet phenomenon: already trans people are vestry members, Deputies to General Convention, Eucharistic ministers or Lectors; already, transgender people are priests and deacons in a handful of dioceses in this church. But now we affirm and underscore that practice. Transgender people are not just in Massachusetts, Washington State, and California. We are, as the saying goes, everywhere.
We knew that the resolutions were on the Deputies' calendar for the day, so a number of TransEpiscopal members listened in the gallery, once more on the edge of our seats.
As the House moved quickly down their calendar list, our resolutions quickly approached. But just as D019 came up, a problem emerged. A combination of factors had caused a delay in the Spanish translation of several complex resolutions. As a result, the House would need to delay the vote until at least the afternoon session, maybe longer.
We adjourned to Steak n' Shake.
After a raucous lunch (pressure release being a good and necessary thing) we said goodbye to Tina Beardsley who was flying back to the UK. We very much miss her and so appreciated her warmth and wry humor—by the end of her stay, Tina and roommate Rev. Gari Green had practically developed a Midwest/UK vaudeville act.
Back in the Deputies gallery, D019 quickly came to the floor. Once more, backers were ready to roll. We heard from Sarah Lawton of the Diocese of California, whose sister is trans. We heard from Deputy Dante Tavolaro, transman from Rhode Island. We heard from Rev. Carla Robinson, transwoman from the Diocese of Olympia. From a bevy of young adults, including Sam Gould from the Diocese of Massachusetts, and Natalie Venatta of the Diocese of Kansas. A Deputy from Alaska spoke of trans people in his congregation. There were innumerable allies, just as in the hearing before the Ministry Committee. People from across the United States—all manner of regions, and not simply the coasts—stood up and spoke passionately in support. There were some people opposed to the move, and they were more represented on the floor of the House than in the hearing, though still a clear minority. As expected – and as happened in the House of Bishops in 2009 – they tried to amend the resolution to remove the specific language from the canon. In support of this move, a Deputy from the Diocese of Albany ridiculed the growing list of protected categories, saying she felt slighted "as a red-head" for not being included despite being a minority of the population. My mom and sister are both red heads. I can only imagine how fiercely they would have responded to that comment.
In any case, the supportive Deputies were more than ready for the amendment, and it was soundly defeated. A vote on the original resolution followed quickly, and at 3:15pm it passed by a landslide. Debate had lasted for a half hour.
D002 came up directly afterward. In many ways, as in the House of Bishops, the debate was a continuation of the previous one. The amendment tactic having failed, however, it was not tried again. Once more Deputies from all around the church, North and South, Midwest, East and West, got up and spoke in support. Sarah Lawton of California spoke of her experience with trans clergy, saying we as a church will be "richly blessed" if we open our ordination process explicitly to trans people. Carla Robinson spoke of the rigorous process she underwent for ordination in the Diocese of Olympia, even after having been ordained in the Lutheran Church, Missouri Synod. She wanted to make the supportive atmosphere she experienced in that process more widely accessible. Then a Deputy from Alabama in a plaid sport coat and bow tie (in honor of Gregory Straub, Secretary of the General Convention, who is known for his crazy sport coats) got up and began speaking. At first I couldn't tell if he would speak in favor or against. But then he said that we are to make God's kingdom present here on earth, and read from Isaiah 56:4-5:
For thus says the Lord:
To the eunuchs who keep my sabbaths,
who choose the things that please me
and hold fast my covenant,
I will give, in my house and within my walls,
a monument and a name
better than sons and daughters;
I will give them an everlasting name
that shall not be cut off.
These were a people, he said, that formerly had not been allowed access to the assembly. They had been a people cut off—unwelcome because of what we might refer to as their gender identity and expression—but now they were welcomed. "We must name what God has named," he said.
TransEpiscopal members were sitting in a row in the gallery. When he said that, we all just lost it. I tweeted
#GC77 Dio Ala: we r to establish kingdom here on earth, now. Let not eunuch say I am a dry tree (Is 60); we must name what God has named
#GC77 Dep from Alabama: wow, you absolutely made my day #TransEpiscopal
Shortly thereafter, debate finished. Again, as expected, and as happened in 2009, a Deputy (Diocese of Albany) requested a vote by orders. This tactic makes it more difficult to pass legislation. Instead of a voice vote, in which a simple majority suffices, a vote by orders tabulates by each diocesan deputy team (what's called a Deputation). The votes of evenly divided deputations count as "no" votes. The most contentious resolutions tend to be tabulated in this way. It also delays the results, as they must be certified. So, as Deputy business continued, we waited. We stood up and sang "Be Thou My Vision." A fifteen minute recess came and went. Still no results. We were on the edge of our seats once more. Finally, a question emerged as to when we would hear the results. Secretary Straub let President of the HoD Bonnie Anderson know that she had the results already. No, she said, she had not yet received them. But then—aha!—she realized they had been before her for some time. All of us seated in the gallery roared.
She read them aloud: we had done it. A landslide.
At 4:48pm I tweeted:
#GC77 D002 PASSES!!!! By a lot!!!
#GC77 D002: Y lay: 94; Y clg: 95; N lay: 11; no clg: 16; Divided lay: 5; Divided clg: 0; thus, No + Divided lay: 16; No + Divided clg: 16
It had passed by 85%.
We were Transfigured.
**Photos by Anderson C (except photo #2)
Posted by Cameron Partridge at 12:14 PM
Labels: D002, D019, General Convention, House of Deputies, TransEpiscopal, transgender clergy, transgender nondiscrimination legislation
Summary of the Acts of the 77th General Convention
Meant To Be Transfigured
Healing Waters
Edge of Our Seats
The Listening Process Compared
A Church Where All Can Actually Mean All
Slingshot Ministry at the 77th General Convention:...
D019 Testimony from Donna Cartwright
Hearing on D002 and D019 -- Powerful Witness
General Convention 2012: Off and Running


The organizing committee of the Malware Conference is delighted to announce that for its 10th year anniversary Prof. Vern Paxson, from the University of California at Berkeley, will serve as our Keynote speaker. Dr. Paxson is a fellow of the Association for Computing Machinery (ACM), and a well know and highly respected researcher in the fields of Internet measurement and Internet security. Vern will be sharing with us his perspective on Broad Spectrum Attacks, what is to be expected in the future, and some new work that his research organization is currently pursuing.
network activity and Internet attacks. He has worked extensively on high performance network monitoring and on cybercrime, and co-directs the Center for Evidence-based Security Research (www.evidencebasedsecurity.org).
In 2006 Paxson was inducted as a Fellow of the Association for Computing Machinery (ACM). The ACM's Special Interest Group on Data Communications (SIGCOMM) gave Paxson its 2011 award, "for his seminal contributions to the fields of Internet measurement and Internet security, and for distinguished leadership and service to the Internet community." The annual SIGCOMM Award recognizes lifetime contribution to the field of communication networks.
He is also a recipient of the ACM's Grace Murray Hopper Award, and the 2015 IEEE Internet Award.


When I shared my personal struggles with body image, the response was staggering. I was amazed by how many women and young girls were silently suffering. I was overwhelmed by your emails, your comments, your kind words – the resounding "me too" and "thank you for letting me know I'm not alone." And while at first I felt validated, those feelings quickly turned to anger. Our generation has been duped. We've been lied to and manipulated. Our very psyche has been tampered with – we have been programmed to never be happy with the way that we look – all for someone else's bottom line.
Think about it: How many BILLIONS of dollars would be lost if every woman woke up tomorrow and believed that she was beautiful? That she wasn't some work in progress, that her body wasn't in constant need of improvement? This about how much money is made by making women feel inferior.
We're taught to never be happy – to never feel good about ourselves.
I'm telling you that it is a LIE. An ugly, greedy, manipulative lie. And I say enough is enough.
I'm fed up. I refuse to let another generation be led to believe the LIES that we have been taught to believe. Let's not let our daughters grow up in a world where they never feel pretty enough or skinny enough. Let's create a world for them in which their diversity is their greatest strength – a world where women are valued for their minds, their hearts, and their deeds. Where individuality is celebrated, where media portrayals are honest, healthy depictions of real women. Let's put an end to the lies.
I have created the #NoMoreLies movement to challenge narrow socially constructed ideas of beauty, demand a more healthy, real, and diverse portrayal of women in the media, and teach women and young girls to love their bodies, break the cycle of hate, and stop believing the lies.
Dual Audience: 1. Women – policy changers, mothers, those directing the social climate/popular culture – those who can make a difference in their homes, their schools, their communities. 2. Young girls – who can be taught the WHY behind society's obsession with physical perfection, who can be taught how to be healthy: mentally and physically, who can be taught to separate self esteem from physical attractiveness.
Encourage beauty – not socially constructed ideas of beauty, but the broader sense of beauty in all women – the beauty of our spirits, our works, our ideas – and seeing a reflection of these ideals widely embraced by popular culture.
Promote healthy eating and exercise.
End the physical objectification of women and the cultural obsession with perfection.
End use of highly photoshopped images. You're never going to look like the girl in the magazine because the girl in the magazine doesn't look like the girl in the magazine. It. Isn't. Real.
Stop programming women to strive for unrealistic, idealized constructs of beauty – we are TAUGHT to never be happy with our appearance with our bodies all for someone else's PROFIT – someone else's bottom line. We are being objectified and controlled. Enough is enough.
Understand that there will always be pretty girls, and skinny girls, and social norms for what is considered attractive, but to be able to recognize beauty is much broader than we have been lead to believe and that physical attractiveness is just a tiny piece of who we are.
We're talking about creating a dramatic shift in our culture – one that won't be easy – but wouldn't it be nice if our daughters could grow up in a world where their wasn't an obsession with physical perfection? Where women were valued for their minds, their hearts, and their contributions to society? Where we could see beauty in every type of woman? Where we could see beauty in ourselves each an every day in each and every season of our lives?
1. Link up your story. Have you struggled with body image? Are you ready to make a commitment to start loving yourself and be a better example for the next generation? Add your body image post to the link up below and be sure to use the hashtag #nomorelies and link to this page for people to go for more information.
2. Use #nomorelies on social media when sharing pieces that promote positive self image, expose media bias and societal pressures, and encourage true, diverse and meaningful beauty.
3. Become an advocate. Reach out to your local communities, schools, churches, and parenting groups. Plan events. Lobby for better self-esteem/body image/media bias education for young girls. Reach out to other bloggers, print publications and online magazines. Let your voice be heard. It's time to speak up. It's time to make a difference.
4. E-mail me with your ideas, thoughts, and success stories. Share resources. Let's do this together. I can be reached via my contact page or at fcfashionista at gmail dot com.
Let's put an end to the lies. Let's stop telling them. Let's stop believing them.


On Monday evening the students at Bath Academy of Musical Theatre were treated to an inspiring masterclass with West End and TV star Helena Blackman.
Helena trained at GSA and is best known following her appearance on the BBC1 show 'How Do You Solve A Problem Like Maria'. She has since performed in many West End and touring musicals including The Sound Of Music, South Pacific, Gypsy and The Wizard of Oz. She has worked with many of the biggest names in theatre – including Julia McKenzie, Ian McKellen and Andrew Lloyd Webber.
Each of the BAMT students was given the opportunity to perform for and work with Helena on either a monologue or musical theatre song.
Founded by Rob Hickmore and Tim King, Bath Academy of Musical Theatre is now in its second year offering the best musical theatre training in the area. The course focusses on audition preparation and is a must for anyone wishing to gain entry to full time drama school and musical theatre courses.
Due to Rob and Tim's connections with the West End and top drama schools, students at Bath Academy of Musical Theatre are regularly treated to masterclasses with highly experience performers and directors, such as Mary Hammond (Royal Academy of Music), David Ashley (Cats, Blood Brothers), Helen Colby (Sweeney Todd and Sister Act) and Neil Ditt (Mary Poppins and High Society).
Bath Academy of Musical Theatre will be offering a Free Taster Session on Monday 8th April to anyone interested in attending the course. The evening will include practical workshops in singing, dance and acting – and is an ideal opportunity to meet the staff. This event will be followed by the first set of auditions on 29th April for entry in September 2013.