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Reality Star-in-Chief
by Paul Gleiser · Published December 13, 2018 · Updated December 16, 2018
AP Photo/Evan Vucci
Think back to the 2012 presidential campaign and Mitt Romney. As you may recall, the Democrats and their media enablers very successfully painted Romney as a rich, out-of-touch 'one percenter' who could never possibly understand the concerns of 'ordinary Americans.' In response, Romney fecklessly treated us to home movies of himself and his family loading up the station wagon and going on vacation.
See, I'm not rich.I'm just an ordinary family guy.
It didn't work. Romney was never able to shake the media-created image of silver spoon Brahmin. The Richie Rich meme stuck to Romney like a wet suit.
With that recollection in mind, jump ahead to June 2015. In the first few minutes of his announcement for the presidency, Donald Trump, in making the point that his presidency wouldn't be beholden to PACs and big-money lobbyists said, "I'm really rich." In an instant, and even though Donald Trump is by several multiples more wealthy than Mitt Romney, the issue of wealth was off the table. The Dems and the media never raised it once because they knew that if they tried, it wouldn't work. Many times throughout the campaign Trump bragged on his personal wealth with complete impunity. Working class stiffs voted for him in sufficient numbers to lead him to an upset victory over the heavily-favored Hillary Clinton.
Taking that recollection, jump further forward to this past Tuesday. Sitting in the Oval Office with Democrats Nancy Pelosi, who will be Speaker of the House in about three weeks, and Senate Minority Leader Chuck Schumer – and with the cameras rolling — the president loudly and proudly said that he would be perfectly willing to shut down the government if the next funding bill didn't include money for his border wall.
Just like that, Trump ripped from their hands the cudgel that Democrats have used on Republicans at every budget impasse. "I will take the mantle of shutting down, and I'm going to shut it down for border security," said the president. It was a master stroke of reality TV from the master of the genre.
Of course, the media is sputtering and fuming and carrying on. But let them. Every second of air that they give to the story further cements in the minds of those who voted for him that Trump means to keep his promise. He ran on stopping illegal immigration. He ran on building a border wall. If it constitutes the only leverage he has to keep those promises, a government "shutdown" is a feature, not a bug. ("Shutdown" is in quotes because we have learned from prior "shutdowns" that the federal government is so all-pervasive that it cannot actually be shut down.)
In one move, Trump outed the Democrats as the open border advocates that they are while simultaneously giving cover to Congressional Republicans (if they're smart enough to use it).
It was a Trump tour de force. And if it's any indication, it portends a long two years for soon-to-be Speaker Pelosi.
Tags: budgetchuck schumerdonald trumpgovernment shutdownnancy pelosi
The media's epic fail on immigration.
by Paul Gleiser · Published June 21, 2018 · Last modified June 29, 2018
For once, Jim Hoffa is right.
Step away from the Big Gulp, ma'am!
by Paul Gleiser · Published May 31, 2012 · Last modified June 1, 2012
Holland Cooke says:
JUST in time for Christmas.
What a mensch.
Buddy Saunders says:
That open to the media meeting was just what we needed. Nice to see Pelosi and Schumer try to peddle their poison in public. Two rats smoked out!
The two Bushes rarely made me proud of them. Not since Reagan, not until President Trump, has there been a president I have been happy with. President Reagan was a man who strove to deliver on his promises. And now we have President Trump who is delivering on promises made, despite an unprecedented elitist headwind. Donald Trump is not the perfect man, nor the perfect president, but he is the man the nation needs. He is delivering on what he promised those of us who voted for him. If fixing illegal immigration and getting the funding for our border wall requires shutting down the government, then let's do it, Mr. President, let's do it.
Wider-angle shot: Trump is less an issue than a symptom:
https://www.usatoday.com/story/opinion/2018/12/13/donald-trump-executive-power-president-war-democracy-constitution-cult-column/2065368002/
Mr. Cook, your "wide-angle shot" goes wide of the mark. President Trump is neither an "issue" nor a "symptom." He is a man doing what we who voted for him elected him to do.
Mr. Saunder, would you wager cash that The Wall will be built?
Trace Havard says:
No, I don't think it ever will be, I hope I'm wrong and I truly believe this is the final opportunity to get it done, but on the left you have open border advocates more interested in future votes than the American people they are supposed to serve. On the right you have just enough politicians beholden to the cheap labor lobbyists.
And in the center you have the American Middle and lower Middle Class who bear the brunt of paying for the Dems federal largess to illegals and whose paychecks increasingly slide downward due to the cheap labor..
Richard Anderson says:
I agree Mr. Saunders. President Trump is doing the things that others talked about doing, but never followed thru with ACTION. He is.
Same question.
Don't need to wager* (*i.e. gamble cash money just for the sake of propping up my convictions like you apparently feel you need.)
In answer to the core of your question however, do I think THE WALL will be built?
YES, 100%, because the Angel Families who have lost countless loved ones to foreign nationals being in the U.S. illegally, has caused such a public outrage, as well as the illegal drugs pouring thru wide open border spaces, and numerous other reasons, the public outcry has reached such a level, that now even National Security is on the line, and those few individuals "in high & low places" who still oppose a wall, cannot provide any logical answer which can bear up under scrutiny when Israel has built such a wall and proven that it brought near total impenetrability to a border that was once wantonly violated by terrorists, but no more.
REMEMBER THIS, go back and look at the various video montages of the nattering nabobs of negativism, the pundits, the prognosticators, the poobahs, who laughed at "the very idea of President Trump even becoming the Republican nominee" let alone winning the 2016 election. Well, to be sure, going back to his announcement, I was not one them, nor were the millions of citizens in thousands of counties across America who voted Donald J. Trump into office. And we're going to do it again in 2020.
The perpetual "Hate Trump" Marxist religion is determined to take down our duly elected Trump Presidency by any means necessary with lies, half-truths, and deception. What we freedom-loving and Constitution advocates are watching today, in real time, is a coup d'état by the Left with saturation propaganda bombing using verbal/video/media/blog outlets at every opportunity, all in the "name" of free speech, of course. Our "free speech rights" gives the Left the right to persuade an ignorant citizenry to put their faith in the evil Left whose goal is to destroy our freedoms, one slice at a time. Once the Left wins, of course, all freedom disappears and there will be NO "free speech" or any other rights as granted by God and protected by the Constitution. The following video puts this political coup in context as discussed by real Patriots that are fearless to expose the agenda of the Left and its subversive followers.
"The Scandal of Our Generation": https://www.youtube.com/watch?v=4KPMgKvJZ88
I believe that Trump is aware of the enemy at the door and is cleverly planning (with God's help) to expose, in due time, the evil in our government and government supported institutions. If not, the march of the Left towards a Marxist America for the last 80 years will have been successful and like a "black hole," the epoch of "The Enlightenment" will be sucked into everlasting darkness with the tyranny of the Middle Ages returning to enslave the masses. This may be our last chance to save ourselves from the tyrannical Leftist hordes.
PREDICTIONS, by those who DO believe The Wall will be built:
Sometimes nagging doesn't engender a response by choice of the nagged who deliberately ignore the nagging with the hope that the nagger will shut up! Those who annoy don't deserve a response because their points are meaningless given the huge scope of danger to the Nation due to the illegal alien invasion that the Marxist Democrats support, ie., NO BORDERS or, Globalism gone berserk.
Why don't you PREDICT the point and time in which Texas will follow California and become a BLUE State after we have absorbed the flow of illegal aliens that have occurred there the last 20 years?
California used to be a very RED State but the LEFT now controls the entire State government and Washington representation. Everyone knows that it is the ILLEGAL ALIEN invasion that is the hope and plan of the Marxist Democrat Party to subvert the Constitution by attracting this illegal flow (dependent on government largess as victims of socialism and BIG government) to eventually overwhelm the Conservative vote at the polls. (Yes, illegal aliens vote in California with illegal support of the Democrat Party.) Once Texas and Florida go BLUE and Leftist tyranny succeeds, there will never be another Republican President, followed eventually by a one Party, Marxist Democrat Congress.
Toleration of the illegal alien invasion erases our borders and destroys our free-market, free-enterprise, Constitutional system. Upon completion of this trend, the Left will have finally taken over our Nation and our Rights will become history. I predict less than 10 years. What's your prediction?
As to your specific question: Experience dictates that the quickest way to induce yawns is to say the word "demographics," because numbers are less sexy than claims. That said: Texas demography is already DANG close to purple.
And just moments ago, a Republican congressman from Texas predicted on TV: NO shutdown. "We'll get a C.R."
Ironically, the next congressman interviewed, from the Democratic House leadership, thought we might GET a shutdown, the-undoing-of-which will be the first piece of business the new Congress takes up.
One thing today has made clear: Trump LISTENS to Rush. ;)
And if you can't wait for Mexico to pay for it:
https://www.gofundme.com/TheTrumpWall
Next story Keep Christmas well.
Previous story Days of merry and bright.


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Homo Sacer: Sovereign Power and Bare Life Giorgio Agamben | EBOOK
The work of Giorgio Agamben, one of Italy's most important and original philosophers, has been based on an uncommon erudition in classical traditions of philosophy and rhetoric, the grammarians of late antiquity, Christian theology, and modern philosophy. Recently, Agamben has begun to direct his thinking to the constitution of the social and to some concrete, ethico-political conclusions concerning the state of society today, and the place of the individual within it.
In Homo Sacer, Agamben aims to connect the problem of pure possibility, potentiality, and power with the problem of political and social ethics in a context where the latter has lost its previous religious, metaphysical, and cultural grounding. Taking his cue from Foucault's fragmentary analysis of biopolitics, Agamben probes with great breadth, intensity, and acuteness the covert or implicit presence of an idea of biopolitics in the history of traditional political theory. He argues that from the earliest treatises of political theory, notably in Aristotle's notion of man as a political animal, and throughout the history of Western thinking about sovereignty (whether of the king or the state), a notion of sovereignty as power over "life" is implicit.
The reason it remains merely implicit has to do, according to Agamben, with the way the sacred, or the idea of sacrality, becomes indissociable from the idea of sovereignty. Drawing upon Carl Schmitt's idea of the sovereign's status as the exception to the rules he safeguards, and on anthropological research that reveals the close interlinking of the sacred and the taboo, Agamben defines the sacred person as one who can be killed and yet not sacrificed—a paradox he sees as operative in the status of the modern individual living in a system that exerts control over the collective "naked life" of all individuals.
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redpajama_set_name: RedPajamaCommonCrawl


text:
\section{Introduction}
\label{sec:intro}

The two-dimensional (2D) Edwards-Anderson spin-glass model
\cite{EA-75} has been extensively studied in recent years in order to
investigate the interplay of disorder and frustration in 2D systems.
If frustration is sufficiently large, these systems are paramagnetic
at any finite temperature $T$.  A critical glassy behavior is only
observed for $T\to 0$. The zero-temperature behavior has been
extensively studied. It is now well understood that it depends on the
behavior of the low-energy spectrum. One should indeed distinguish
systems with a discrete energy spectrum (DES), such as the $\pm J$ Ising
model with a bimodal coupling distribution, from systems with a
continuous energy spectrum (CES), such as the Ising model with Gaussian
distributed couplings \cite{AMMP-03,JLMM-06,LMMS-06}. At $T=0$, these
two classes of systems behave quite differently. For instance, in DES
systems, the stiffness exponent vanishes, while in CES systems, we have
$\theta < 0$; recent numerical studies \cite{footnote-theta} give
$\theta \approx -0.28$.

For finite values of $T$, CES systems show a standard critical
behavior, consistent with what is observed at $T = 0$. In particular,
one expects $\nu = -1/\theta$ and $\eta = 0$, two predictions which
are consistent with numerical data \cite{JLMM-06,KLC-07}. The behavior
of DES systems is instead more complex. In a finite box of linear size
$L$, one observes two different behaviors, which depend on how large
$L$ is compared to a temperature-dependent crossover length $L_c(T)$;
see Refs.~\cite{JLMM-06,THM-11a,THM-11b,JK-11,PPV-10} and references
therein.  For $L< L_c(T)$, the critical behavior is analogous to that
observed at $T=0$. The system shows an effective long-range spin-glass
order and its critical behavior can be predicted using droplet
theory \cite{THM-11a,JK-11}.  On the other hand, for $L>L_c(T)$, the
system is effectively paramagnetic.  Equivalently, at fixed $L$, one
observes the two regimes for $T<T_c(L)$ and $T>T_c(L)$, respectively,
where $T_c(L)$ is the corresponding crossover temperature. Note that
this discrete behavior can only be observed for finite values of $L$,
since $T_c(L)\to 0$ for $L\to\infty$.
Of course, since $T_c(L)$ is an effective finite-size temperature,
the crossover temperature is not uniquely defined,
and many different definitions can be used.
One of the basic questions is whether the critical behavior
of DES systems for $T>T_c(L)$ is the same as that observed in CES
systems. The numerical results of Ref.~\cite{JLMM-06} strongly
suggested that this is the case.  However, those conclusions were
later questioned in Ref.~\cite{KLC-07}, on the basis that much larger
lattices were needed to show it conclusively.

In a renormalization-group (RG) picture, the two regimes can be
interpreted as due to two different fixed points (FPs)
\cite{JLMM-06,JK-11}: a stable FP---the same that controls the
critical behavior of CES systems---which describes the infinite-volume
behavior up to $T=0$, and an unstable FP, present only in DES systems,
which controls the low-temperature behavior for $T < T_c(L)$.

In order to fully specify the two regimes, one should predict how
$T_c(L)$ scales with the size $L$.  A free-energy argument, based on the
energy difference and degeneracies of the two lowest-energy states~\cite{KLC-07}, suggests $T_c(L)\sim 1/\ln L$ as $L\to
\infty$. However, recently, using droplet theory,
Refs.~\cite{THM-11a,THM-11b,JK-11} suggested a power-law behavior
\begin{equation}
L_c(T)\sim T^{-1/\theta_S}, \qquad\qquad
T_c(L) \sim L^{-\theta_S}.
\label{TcL}
\end{equation}
Reference \cite{THM-11a} predicted $\theta_S \approx 0.50(1)$,
which appears to be consistent with their numerical data for the
twist free energy \cite{THM-11a} and the two-point correlation function
\cite{THM-11b}, as well as with previous results \cite{SK-94,LMMS-06}.
A calculation in a hierarchical model \cite{JK-11} gives
a similar result of $\theta_S \approx  0.37$.
These calculations indicate that although $\theta_S$ is quite small,
it is nonetheless larger than the exponent $1/\nu = -\theta \approx 0.28 $
($\theta$ is the stiffness exponent in CES systems).

In this paper, we investigate again the question of universality, by
comparing the finite-size scaling (FSS) of the $\pm J$ model for two
values of the disorder parameter $p=0.5,\,0.8$ and the model with
Gaussian distributed couplings (henceforth we call it the Gaussian model).
The FSS analysis in terms of RG invariant quantities (for example, the
plots of the Binder cumulants versus the ratio $\xi/L$, with all quantities
being defined in terms of the overlap variables) shows that the two
models belong to the same universality class, confirming the
conclusions of Refs.~\cite{JLMM-06,LMMS-06}. Indeed, the $\pm J$ data
have the same FSS behavior as the Gaussian data, if we only consider
the $\pm J$ model results corresponding to temperatures larger than
the crossover temperature.  Then, we focus on the validity of the
standard FSS in terms of the variable $TL^{1/\nu}$, which is a rather
subtle point in DES systems.  Standard FSS exists only if
$T_c(L)L^{1/\nu}\to 0$ for $L\to \infty$.  If we assume $T_c(L)\sim
L^{-\theta_S}$, then since $T_c(L)L^{1/\nu} \sim L^{1/\nu - \theta_S}$, FSS
can be observed only if $\theta_S > 1/\nu\approx 0.28$.  This implies
that if $T_c(L) \sim 1/\ln L$
\cite{KLC-07,PPV-10}, the FSS limit $T\to 0$, $L\to\infty$ at
fixed $TL^{1/\nu}$ does not exist in DES systems.  On the other hand,
if Eq.~(\ref{TcL}) holds with $\theta_S \approx 0.50$, FSS holds also
in DES models.  However, the approach to the asymptotic limit is quite
slow. The region in which no FSS is observed, which corresponds to
$TL^{1/\nu} \lesssim T_c(L)L^{1/\nu}$, shrinks slowly, as $L^{1/\nu -
\theta_S}\sim L^{-0.2}$.  The comparison of the Monte Carlo (MC)
simulations of the $\pm J$ and Gaussian models shows quite
convincingly that for fixed $TL^{1/\nu}$ close to $T_c(L) L^{1/\nu}$,
the $\pm J$ model data converge toward the data of the Gaussian
model, confirming the existence of the standard FSS, hence the
power-law behavior (\ref{TcL}) with $\theta_S > 1/\nu$. A reanalysis
of the freezing temperature $T_f(L)$, defined in Ref.~\cite{PPV-10}
from the freezing of $\xi/L$ and of the Binder cumulants [at fixed $L$,
they are approximately constant for $T<T_f(L)$], is consistent with
Eq.~(\ref{TcL}) with $\theta_S \approx 0.4$, which is close to the
estimate of Ref.~\cite{THM-11a}. The freezing temperature $T_f(L)$
should represent a correct effective definition for $T_c(L)$, although
deviations from the universal FSS behavior are expected for somewhat
larger values of $T$.

We also investigate the FSS behavior of the magnetization and the
two-point correlation function of the overlap variables. We find that
the data are consistent with the hyperscaling relation $2\beta=\eta\nu$.
However, the data are not sufficiently precise to provide a precise
determination of $\eta$, being consistent with a small value of
$\eta\lesssim 0.2$, including $\eta=0$.  In Ref.~\cite{THM-11b}, the
authors showed that a properly subtracted overlap correlation function
scales in the temperature region they consider, which essentially
corresponds to $T\lesssim T_c(L)$. Here we consider the opposite regime, $T >
T_c(L)$.  We find that standard FSS as well as universality hold for
the overlap correlation function.

The paper is organized as follows. In Sec.~\ref{sec:mc}, we define
the models and the quantities we investigate. Section \ref{sec:results}
reports the numerical results of our FSS analysis: in
Sec.~\ref{sec3.1}, we discuss the RG invariant couplings, such as the
ratio $\xi/L$ and the cumulants of the overlap variable, focusing
mainly on the question of the validity of FSS in terms of
$TL^{1/\nu}$; in Sec.~\ref{sec3.2}, we discuss the overlap
magnetization and susceptibility; and finally, in Sec.~\ref{sec3.3},
we discuss the two-point correlation function. In Sec.~\ref{sec4}, we
present our conclusions.

\section{Models and definitions}
\label{sec:mc}

We consider the 2D Ising model on a square lattice with Hamiltonian
\begin{equation}
{\cal H} = - \sum_{\langle xy \rangle} J_{xy} \sigma_x \sigma_y,
\label{lH}
\end{equation}
where $\sigma_x=\pm 1$, the sum is over all pairs of lattice
nearest-neighbor sites, and the exchange interactions $J_{xy}$ are
uncorrelated quenched random variables.  We consider a model
with Gaussian bond distribution,
\begin{equation}
P(J_{xy}) \sim \exp (-J_{xy}^2/2)
\label{gaudistr}
\end{equation}
(in the following, we call it the Gaussian model).
We also consider the $\pm J$ model where the
couplings $J_{xy}$ take values $\pm J$ with probability distribution
\begin{equation}
P(J_{xy}) = p \delta(J_{xy} - J) + (1-p) \delta(J_{xy} + J).
\label{probdis}
\end{equation}
As in Ref.~\cite{PPV-10}, we consider $p=0.5$ and $0.8$.  We recall
that for sufficiently large frustration, i.e.,
for $0.11 \lesssim p \lesssim 0.89$,
the model shows a zero-temperature glassy critical behavior, with
a paramagnetic low-temperature phase.
Ferromagnetism can only be observed
for $p>p^*=0.89093(3)$ \cite{PPV-09}.

The critical modes at the glassy transition are those related to the overlap
variable $q_x \equiv \sigma_x^{(1)} \sigma_x^{(2)}$, where the spins
$\sigma_x^{(i)}$ belong to two independent replicas with the same disorder
realization $\{J_{xy}\}$.  In our Monte Carlo (MC) simulations, we compute the
overlap magnetization
\begin{equation}
  m = \frac{1}{L^2} [\langle|\sum_x q_x|\rangle],
\end{equation}
the overlap susceptibility $\chi$, and the
second-moment correlation length $\xi$ defined from the correlation
function
\begin{equation}
G_o(x) \equiv [\langle q_0 \,q_x \rangle] =
[\langle \sigma_0 \,\sigma_x \rangle^2],
\label{go}
\end{equation}
where the angular and the square brackets indicate the thermal average
and the quenched average over disorder, respectively. We define $\chi
\equiv \sum_{x} G_o(x)$ and
\begin{eqnarray}
\xi^2 \equiv  \frac{1}{4 \sin^2 (p_{\rm min}/2)}
\frac{\widetilde{G}_o(0) - \widetilde{G}_o(p)}{\widetilde{G}_o(p)},
\label{xidefffxy}
\end{eqnarray}
where $p = (p_{\rm min},0)$, $p_{\rm min} \equiv 2 \pi/L$, and
$\widetilde{G}_o(q)$ is the Fourier transform of $G_o(x)$.  We also
consider some quantities that are invariant under RG transformations
in the critical limit, which we call phenomenological couplings.  We
consider the ratio $\xi/L$ and the quartic cumulants
\begin{equation}
U_{4}  \equiv \frac{[ \rho_4 ]}{[\rho_2]^{2}}, \quad
U_{22} \equiv  \frac{[ \rho_2^2 ]-[\rho_2]^2}{[\rho_2]^2},
\label{uc}
\end{equation}
where $\rho_{k} \equiv \langle \; ( \sum_x q_x\; )^k \rangle$.

In the case of a $T=0$ transition with a nondegenerate ground state,
as expected in CES systems, the overlap magnetization
exponent $\beta$  vanishes, and
$U_{4}\to 1$ and $U_{22}\to 0$ for $T\to 0$. Moreover,
assuming the hyperscaling relation $2\beta = \eta\nu$, we obtain $\eta=0$, thus
$\chi\sim \xi^2$ for $T\to 0$.

\section{Finite-size scaling behavior}
\label{sec:results}

In order to study the FSS behavior, we extend the MC simulations of
the $\pm J$ model at $p=0.5$ and $0.8$ presented in
Ref.~\cite{PPV-10}; we perform further simulations of the $\pm J$
Ising model at $p=0.8$ on finite square lattices of sizes $L=16,32$,
and of the Gaussian model for $L = 8,12, 16$.  We use the Metropolis
algorithm and the random-exchange method~\cite{raex}.  For the
Gaussian model, we study the temperature interval $T_{\rm min}\le T
\lesssim 1.6$, with $T_{\rm min}=0.2$ ($L=8$) and $T_{\rm min}=0.167$
($L=12,16$). We average over a large number of disorder samples, i.e.,
$10^4$ for each $T$ and $p$.

\subsection{RG invariant couplings} \label{sec3.1}

To begin with, we wish to check that the $\pm J$ model and the
Gaussian model belong to the same glassy universality class, extending
the FSS analyses of Refs.~\cite{JLMM-06,KLC-07,PPV-10}.  For this
purpose, we consider $U_4$ and $U_{22}$ as a function of $\xi/L$. Our
numerical results for the largest values of $L$ are reported in
Fig.~\ref{FSSxiL}. No scaling corrections are visible in the plot of
$U_4$, as already observed in Refs.~\cite{KLC-07,PPV-10}, while
slightly larger corrections appear in the case of $U_{22}$ for $\xi/L
\gtrsim 0.6$. It is, however, evident that as $L$ increases, the
differences between the Gaussian model results and those for the $\pm
J$ model decrease.  Thus, these results, together with those presented
in Refs.~\cite{JLMM-06,KLC-07} (in Ref.~\cite{JLMM-06}, other CES and
DES systems were considered), confirm that all models belong to the
same universality class.

\begin{figure}
\includegraphics[width=17em,keepaspectratio]{rxiu4.eps}
\hspace{1truecm}
\includegraphics[width=17em,keepaspectratio]{rxiu22.eps}
\caption{(Color online)
The cumulants $U_4$ and $U_{22}$ vs
$\xi/L$.  We present data for the $\pm J$ model ($p= 0.5$ and $0.8$)
and for the Gaussian model. Only the data for the largest lattices are
included for clarity.
}
\label{FSSxiL}
\end{figure}

Now we investigate the question of the existence of standard FSS as
a function of $T L^{1/\nu}$. For a RG-invariant quantity $R$, we expect
\begin{equation}
   R = h_R(x), \qquad\qquad x \equiv a T L^{1/\nu},
\label{RFSS}
\end{equation}
where $a$ is a nonuniversal constant that depends on the model
but not on the quantity $R$, which can be chosen so that $h_R(x)$ is
model independent.

\begin{figure}
\begin{tabular}{cc}
\includegraphics[width=18em,keepaspectratio]{rxitgau.eps} &
\includegraphics[width=18em,keepaspectratio]{u22tgau.eps} \\
\includegraphics[width=18em,keepaspectratio]{rxit0p5.eps} &
\includegraphics[width=18em,keepaspectratio]{u22t0p5.eps} \\
\includegraphics[width=18em,keepaspectratio]{rxit0p8.eps} &
\includegraphics[width=18em,keepaspectratio]{u22t0p8.eps} \\
\end{tabular}
\caption{(Color online) The phenomenological couplings $\xi/L$ (left)
and $U_{22}$ (right) vs $ T L^{1/\nu}$. We report the results for
the Gaussian model (top), and for the $\pm J$ model at $p= 0.5$ (middle)
and at $0.8$ (bottom).  }
\label{FSSstd}
\end{figure}

First, we consider the data for the Gaussian model. The numerical
results for $\xi/L$ and $U_{22}$ are reported versus $T L^{1/\nu}$ in
Fig.~\ref{FSSstd} (top). We use $\nu = 3.55$, which corresponds to
$\theta = - 1/\nu = -0.282$, which in turn is the present best estimate of the
stiffness exponent of the Gaussian model \cite{footnote-theta}.  The
data show that $\xi/L$ and $U_{22}$ scale reasonably as a function of
$T L^{1/\nu}$ and clearly appear to approach a FSS limit with
increasing $L$. Scaling violations increase as $T L^{1/\nu}$
increases.  This is not unexpected since the correct scaling variable
is the combination $u_T(T) L^{1/\nu}$, where $u_T(T)$ is the nonlinear
scaling field associated with the temperature.  Considering $T
L^{1/\nu}$ as the scaling variable corresponds to expanding $u_T(T)$ to
first order in the temperature, an approximation which is expected to
work well only when $T$ is small. On the other hand, the region $TL^{1/\nu}
\gtrsim 2$ corresponds to temperatures $T\gtrsim 1$
for the lattice sizes considered here.
Of course, we cannot exclude the additional presence of
nonanalytic scaling corrections, which increase as $T L^{1/\nu}$
increases.

Then, we consider the data for the $\pm J$ model; see
Fig.~\ref{FSSstd}. The data show essentially three types of behavior,
depending on the value of $TL^{1/\nu}$.  For $TL^{1/\nu}\lesssim 1.5$,
no scaling is observed.  This may be explained by the fact that the
data in this region are below the crossover temperature, i.e.,  they
correspond to $T<T_c(L)$, and thus are outside the regime in which
FSS is supposed to hold. Then, there is an intermediate region, $1.5
\lesssim TL^{1/\nu} \lesssim 2.0$, where data show scaling with small
corrections --- this is particularly evident for $U_{22}$. For
$TL^{1/\nu} \gtrsim 2.0$, the corrections are larger, but the results
appear to rapidly converge  to a limiting curve: for both $\xi/L$ and $U_{22}$, the
results satisfying $L\ge 32$ are very close to each other.  We
conclude that at least for $TL^{1/\nu} \gtrsim 1.5$, FSS apparently
holds.

\begin{figure}
\begin{tabular}{cc}
\includegraphics[width=18em,keepaspectratio]{fssrxiallmo.eps} &
\includegraphics[width=18em,keepaspectratio]{fssu22allmo.eps} \\
\end{tabular}
\caption{(Color online) The phenomenological couplings $\xi/L$ (left)
and $U_{22}$ (right) versus $a T L^{1/\nu}$. We report the results for
the $\pm J$ model at $p=0.8$ and $0.5$ (only $L\ge 32$) and for
the Gaussian (G) model (only $L\ge 12$).  We fix $a = 1$, $1.5$, and $1.3$ for the Gaussian model, and for the $\pm J$ model at $p=0.8$ and
$0.5$, respectively.  }
\label{FSSstd2}
\end{figure}

Furthermore, we verify the universality of the FSS behavior by
comparing the results for the function $h_R(x)$ defined in
Eq.~(\ref{RFSS}). For this purpose, we should first fix the
model-dependent constant $a$ that appears in Eq.~(\ref{RFSS}).  We
determine it by requiring the FSS curves for $\xi/L$ to coincide in
the region in which $\xi/L\approx 0.5$. Indeed, in this range of
values of $\xi/L$, we observe small scaling deviations in all of the models we
consider. If we set $a = 1$ for the Gaussian model, then for the
$\pm J$ model, we obtain
$a(p=0.5) \approx 1.3$ and $a(p = 0.8) \approx 1.5$.
In Fig.~\ref{FSSstd2}, we plot together the data for the Gaussian model and
the $\pm J$ models at $p = 0.8$ and $0.5$.  For clarity, we only
report the data with $L \ge 32 $ for the $\pm J$ model and the
results with $L \ge 12$ for the Gaussian model. With this choice, there
is only one point (it belongs to the $\pm J$ model with $p=0.8$ and
corresponds to $L=32$) which belongs to the region $T<T_c(L)$. This
point is clearly visible in the figures as an isolated point. If we
discard it, we observe good scaling up to $a T L^{1/\nu} \lesssim
1.5$: the $\pm J$ model data and the Gaussian data fall on top of each
other with good precision.  For $a T L^{1/\nu} \gtrsim 1.5$, the $\pm
J$ data scale reasonably.  The data of the Gaussian model, which correspond
to significantly smaller lattices, show significant scaling
corrections. It is, however, reassuring that the trend is correct: as
$L$ increases, they approach the $\pm J$ results.

In order to understand the behavior close to the crossover temperature
$T_c(L)$, in Fig.~\ref{FSSstd3} we report results for all values of
$L$, but only for $a T L^{1/\nu} < 1.25$. It is clear that the
deviations between $\pm J$ and Gaussian data slowly decrease as $L$
increases (the same occurs for $p=0.5$, not shown). This is consistent with the idea that FSS in terms of $TL^{1/\nu}$ holds asymptotically, and,
hence, with the prediction $T_c(L) \sim L^{-\theta_S}$ with $\theta_S >
1/\nu$.  The approach is, however, very slow. Indeed, the region in
which FSS does not hold is predicted to shrink as
$L^{-\theta_S+1/\nu}\sim L^{-0.2}$.

\begin{figure}
\begin{tabular}{cc}
\includegraphics[width=18em,keepaspectratio]{rximg0p8.eps} &
\includegraphics[width=18em,keepaspectratio]{u22g0p8m.eps} \\
\end{tabular}
\caption{(Color online) The phenomenological couplings $\xi/L$ (left)
and $U_{22}$ (right) vs $a T L^{1/\nu}$ for $a T L^{1/\nu} <
1.25$. We report the results for the $\pm J$ model at $p=0.8$ and for
the Gaussian model.  We fix $a = 1$ for the Gaussian (G) model and $a =
1.5$ for the $\pm J$ model at $p=0.8$. }
\label{FSSstd3}
\end{figure}

\begin{figure}
\begin{tabular}{cc}
\includegraphics[width=18em,keepaspectratio]{tf.eps} \\
\end{tabular}
\caption{(Color online) Log-log plot of the freezing temperature
$T_f(L)$ vs $L$ for the $\pm J$ model at $p=0.8$.  The dashed line
shows a fit to the data, corresponding to $T_f(L)\sim L^{-0.35}$.  }
\label{plotTc}
\end{figure}

This power-law behavior is also supported by the scaling of the
freezing temperature $T_f(L)$ defined in Ref.~\cite{PPV-10}.
For each value of $L$, $\xi/L$ and $U_4$ become constant
for small $T$, assuming values $(\xi/L)_f$ and $U_{4,f}$.
Then, one defines $T_f(L)$ as the largest temperature of the
region in which $\xi/L \approx (\xi/L)_f$ and $U_4 \approx U_{4,f}$.
A fit of the data to a power-law behavior \cite{logw} gives
$T_f(L) \sim L^{-0.35}$; see Fig.~\ref{plotTc}.
Given the {\em ad hoc} procedure \cite{footnote-etf} used to determine
$T_f(L)$, it is difficult to give a reliable error for the result. It is,
however, reassuring that the estimate satisfies the bound $\theta_S >
1/\nu$ and is close to the estimates of Refs.~\cite{LMMS-06,THM-11a}.

\subsection{Overlap magnetization and susceptibility} \label{sec3.2}

The overlap magnetization $m$ and susceptibility are expected to behave
as
\begin{eqnarray}
m = \xi^{-\beta/\nu} u_h(T) f_m(\xi/L),
\label{scalingm}
\end{eqnarray}
and
\begin{eqnarray}
\chi = \xi^{2-\eta} u_h(T)^2 f_\chi(\xi/L),
\label{scalingchi}
\end{eqnarray}
where $f_m(x)$ and $f_\chi(x)$ are universal functions apart from a
multiplicative constant, and the scaling field $u_h(T)$ is an analytic
function of $T$.
If hyperscaling holds, we should have
\begin{eqnarray}
\beta = \frac{\eta\nu}{2} .
 \label{eta-beta}
\end{eqnarray}
Thus, the combination
\begin{eqnarray}
    H = \frac{\xi^2 m^2}{\chi}
\label{defH}
\end{eqnarray}
should be a universal function of $\xi/L$, independent of the scaling
field $u_h(T)$.  In Fig.~\ref{FSSH}, we show the combination $H$ for the
Gaussian model and the $\pm J$ model at $p=0.8$.  The scaling is
good. Deviations are only observed for $\xi/L \lesssim 0.2$ --- these
data correspond to large temperatures --- and for $\xi/L \gtrsim 0.6$,
which, as discussed in Ref.~\cite{PPV-10}, is the region in which
strong crossover effects are observed
for the lattice sizes considered in this paper.
However, the observed trends are consistent with a unique
universal curve. We thus confirm the validity of Eq.~(\ref{eta-beta}),
independently of what the numerical value of $\eta$ is. If, indeed,
$\eta = 0$, as theoretically predicted, Eq.~(\ref{eta-beta}) gives
$\beta = 0$.

\begin{figure}
\begin{tabular}{c}
\includegraphics[width=22em,keepaspectratio]{Hcomb.eps} \\
\end{tabular}
\caption{(Color online) Scaling combination $H$ defined in Eq.~(\ref{defH})
vs $\xi/L$ for the Gaussian (G) model and the $\pm J$ model at
$p=0.8$.
}
\label{FSSH}
\end{figure}

\begin{figure}
\begin{tabular}{cc}
\includegraphics[width=16em,keepaspectratio]{fsschieta0.eps} &
\hspace{1truecm}
\includegraphics[width=16em,keepaspectratio]{fsschieta0p2.eps} \\
\end{tabular}
\caption{(Color online) Scaling combination $\chi L^{\eta-2} u_h^{-2}$
vs $\xi/L$. We report the results for $\eta = 0$ (left) and $\eta
= 0.2$ (right).  Data are for the Gaussian model (G) and for the $\pm J$
model with $p=0.8$ and $0.5$.
}
\label{FSSchi}
\end{figure}

We have fitted all Gaussian data for the overlap susceptibility to
Eq.~(\ref{scalingchi}) --- more precisely to its logarithm as in
Ref.~\cite{PPV-10} --- obtaining $\eta=0.20(7)$.  The error we report
is purely statistical and does not take into account possible scaling
corrections. This result is slightly larger than the predicted result
$\eta = 0$. The discrepancy should not be taken seriously, given the
small lattices we consider.  A precise determination of $\eta$ in the
Gaussian model requires, indeed, much larger values of $L$; see
Ref.~\cite{KLC-07}.

The function $f_\chi(x)$ is universal apart from a rescaling: if
$f_1(x)$ and $f_2(x)$ are determined in two different models, we expect
$f_1(x) = b f_2(x)$, where $b$ is a model-dependent constant. We now
compare the estimates of the functions $f_\chi(x)$ for the Gaussian
model and the $\pm J$ model. In Fig.~\ref{FSSchi}, we report the
functions (they have been rescaled so that they coincide for $\xi/L =
0.3$) for the Gaussian model and the $\pm J$ model at $p=0.8$ and $0.5$. We
report the curves both for $\eta = 0$ and $0.2$. In
Ref.~\cite{PPV-10}, we observed that for $\eta = 0$, the scaling was
good up to $\xi/L\approx (\xi/L)_{\rm max}$, a value which had been
estimated as the boundary of the crossover region before the regime in
which freezing was observed. The quantity $(\xi/L)_{\rm max}$
should scale as $(\xi/L)_{c}$,
i.e., the value of $\xi/L$ at the crossover temperature.
Now, using Eq.~(\ref{RFSS}), since $h_{\xi/L}(x) \sim x^{-\nu}$
for $x\to 0$ to recover the correct infinite-volume behavior, we have
\begin{equation}
(\xi/L)_{\rm max} \sim (\xi/L)_{c} \sim
   h_{\xi/L}[ a T_c(L) L^{1/\nu}] \sim T_c(L)^{-\nu}/L \sim
       L^{\nu\theta_S - 1} \sim L^{0.8},
\end{equation}
where we have used $\theta_S = 0.5$ in the last step, and the fact
that $T_c(L) L^{1/\nu}\to 0$ for $L\to \infty$.
Again note that the inequality $\theta_S > 1/\nu$ is necessary to
guarantee that $(\xi/L)_{\rm max} \to \infty$ as $L\to \infty$.
By looking at the scaling behavior of
$U_{22}$, Ref.~\cite{PPV-10} estimated $(\xi/L)_{\rm max} \approx
0.65$ and $0.45$ for $p=0.8$ and $0.5$, respectively, in the range $32\le L
\le 64$. For the $\pm J$ model at $p=0.5$, a similar estimate is
obtained by considering the scaling behavior of the estimates of
$\xi(2L)/\xi(L)$ reported in Ref.~\cite{JLMM-06}.
The data for the Gaussian model agree with the $\pm J$
model data for both $p=0.5$ and $0.8$ up to $(\xi/L)_{\rm max}$.
Thus, the numerical results are
consistent with universality and $\eta = 0$.

In Ref.~\cite{PPV-10}, we also observed that if we included all data in
the fits, the best estimate of $\eta$ was $\eta \approx 0.2$.  Indeed,
in this case, the results for the overlap susceptibility showed a very
good scaling up to $\xi/L\approx 0.8$.  We did not take this result as
an indication that $\eta = 0.2$ was a more plausible estimate than
$\eta = 0$ because we had good reasons to discard all data beyond
$\xi/L\approx (\xi/L)_{\rm max}$.  Somewhat surprisingly, if we now
include the data for the Gaussian model, and take $\eta = 0.2$ for all
models, we again observe a good universal scaling up to $\xi/L\approx
0.8$.  However, the numerical results of Ref.~\cite{KLC-07} exclude
$\eta=0.2$ for the Gaussian model. Thus, the apparently good observed
behavior cannot hold asymptotically.
In view of the result $\eta=0$ of Ref.~\cite{KLC-07}, as $L$ increases, the Gaussian data should become inconsistent with $\eta = 0.2$.

Finally, we note that,  in order to observe a good scaling behavior for
the overlap susceptibility, it is crucial to include the nonlinear
scaling field $u_h(T)$. Indeed, such a function gives a sizable
contribution to our data. In the case in which we set $\eta = 0$, we
obtain $u_h(T=1)^2/u_h(T=0.2)^2 \approx 2.2$ and
$u_h(T=1.5)^2/u_h(T=0.2)^2 \approx 3.3$.

\subsection{Two-point function} \label{sec3.3}

In Ref.~\cite{THM-11b}, the authors analyzed the scaling behavior
of the two-point function, showing that below the crossover temperature,
the two-point function scales as predicted by droplet theory.
Here we analyze the two-point function in the opposite regime in which
we expect
\begin{equation}
   G_o(r,T) = {\xi^{-2} \chi} f_G(r/\xi,\xi/L).
\label{Gscaling}
\end{equation}
Note that by writing the scaling behavior in this form, there is neither
the need to specify $\eta$ nor to introduce the nonlinear scaling fields.
Moreover, the function $f_G(x,y)$ is universal.

\begin{figure}
\begin{tabular}{cc}
\includegraphics[width=17em,keepaspectratio]{fun2ptL2.eps} &
\hspace{1truecm}
\includegraphics[width=17em,keepaspectratio]{fun2ptL4.eps} \\
\end{tabular}
\caption{(Color online)
Scaling combination $g_o(x,T)$ for $x=L/2$ (left) and $x = L/4$ (right)
vs $\xi/L$. We report results for
the Gaussian (G) model and the $\pm J$ model at $p=0.8$.
}
\label{FSSG_L}
\end{figure}

\begin{figure}
\begin{tabular}{cc}
\includegraphics[width=17em,keepaspectratio]{go.eps} &
\hspace{1truecm}
\includegraphics[width=17em,keepaspectratio]{go0p63.eps} \\
\end{tabular}
\caption{(Color online) Scaling combination $g_o(x,T)$ for
$\xi/L\approx 0.18$ (left) and $\xi/L\approx 0.63$ (right) vs
$x/\xi$. We report the results for the Gaussian (G) model and the $\pm
J$ model at $p=0.8$.  }
\label{FSSG_x}
\end{figure}

To verify the scaling behavior (\ref{Gscaling}), we compute $G_o(r,T)$
along a lattice line, i.e. for $r = (x,0)$. We perform the computation
in the Gaussian model ($L=8,12,16$) and in the $\pm J$ model at
$p=0.8$ ($L=16,32$). Then, we consider
\begin{equation}
   g_o(x,T) \equiv \frac{G_o(r,T) L^2}{\chi}.
\end{equation}
In Fig.~\ref{FSSG_L}, we report $g_o(x,T)$ for $x=L/2$ and $L/4$ as a
function of $\xi/L$, while in Fig.~\ref{FSSG_x}, we show $g_o(x,T)$ at
fixed $\xi/L \approx 0.18$ and $\xi/L \approx 0.63$ as a function of
$x$. In these cases, the scaling is very good: all points fall onto a
single curve, confirming the validity of Eq.~(\ref{Gscaling}) and
universality.

\section{Conclusions} \label{sec4}

We investigate the FSS behavior of two-dimensional Ising spin-glass systems. In particular, we consider the square lattice $\pm J$
model at $p=0.5$ and 0.8, and the Gaussian model.  In this respect,
the $\pm J$ model appears particularly problematic because it
presents two different finite-volume regimes: a {\em continuous}
regime for $T>T_c(L)$ and a {\em discrete} regime for
$T<T_c(L)$. According to droplet theory, the crossover temperature
$T_c(L)$ is expected to vanish in the large-$L$ limit as a power
law~\cite{THM-11a,THM-11b,JK-11}, $T_c(L)\sim L^{-\theta_S}$ with
$\theta_S\approx 0.5$.  A logarithmic behavior, $T_c(L)\sim
1/\ln L$, is instead suggested by the free-energy arguments of
Ref.~\cite{KLC-07}.

The main conclusions of our numerical analysis based on MC simulations
are as follows:
\begin{itemize}
\item[(i)] All models we consider belong to the same universality
class.  The magnetization, susceptibility, two-point correlation
function, and the quartic cumulants, defined in terms of the overlap
variables, show a universal FSS behavior in terms of $\xi/L$.  In the
case of the $\pm J$ model, this universal scaling is only observed above
the crossover temperature $T_c(L)$, which separates the {\em continuous}
region from the {\em discrete} low-temperature behavior.
\item[(ii)] Our FSS analysis provides good evidence of the FSS
limit $T\to 0$, $L\to\infty$ at fixed $TL^{1/\nu}$.  This implies that
the crossover temperature $T_c(L)$ does not behave as $1/\ln
L$ as suggested in Ref.~\cite{KLC-07}, but rather as $T_c(L)\sim
L^{-\theta_S}$ with $\theta_S > 1/\nu \approx 0.28$. This is
consistent with droplet theory, which predicts a
power-law behavior with $\theta_S\approx 0.5$.
 \item[(iii)] We study the FSS behavior of $\chi$.
 The data for the Gaussian and the $\pm J$ models support universality.
 However, the available data are not sufficient to
 obtain a precise estimate of $\eta$ and confirm definitely
 the expected value $\eta=0$.
 \item[(iv)] We verify the hyperscaling relation $2\beta = \eta \nu$.
 If  $\beta=0$, it implies $\eta = 0$.
\item[(v)] We consider the two-point correlation function and show
  that it satisfies a standard FSS ansatz. Note that the scaling form
  (\ref{Gscaling}),
  which is appropriate for a high-temperature phase, is different from
  that considered in Ref.~\cite{THM-11b}, which is appropriate for a
  low-temperature phase in which spontaneous magnetization is present.
  The occurrence of these two different scaling behaviors is related to
  the different regimes considered. Here, we use data such that
  $T>T_c(L)$, while Ref.~\cite{THM-11b} studies the behavior for
  $T<T_c(L)$.
\end{itemize}

redpajama_set_name: RedPajamaArXiv


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LC staff will represent or report for the Library at the following cataloging-related meetings and events during ALA Annual Conference in San Francisco. Information is valid as of June 7, 2001. This listing includes only meetings and events of interest to cataloging staff. For a complete listing of all appearances by LC employees at ALA, see the special LC Web site for ALA, URL http://www.loc.gov/ala/.
The Library's exhibit booth is no. 705, Moscone Convention Center.
LITA Preconference Institute, "The Future of Serials Control: Implementation of the MARC 21 Holdings Format."
Friday, June 15, 8:30 am-5:00 pm, Hilton & Towers, Continental Ballroom 5.
Faculty from LC: Linda Miller (9:45-11:00 am), Rebecca Guenther (11:00 am-12:00 pm).
PCC SACO Workshop A, "Basic SACO."
Friday, June 15, 9:00 am-12:00 pm, Argent Hotel, 50 Third Street, Concordia Room.
Instructor: Lynn El-Hoshy. Preregistration only.
ALCTS Technical Services Directors of Large Research Libraries Discussion Group (Big Heads).
Friday, June 15, 9:30 am-12:30 pm, Marriott-Salon 9.
PCC SACO Workshop B, "Ethnic Groups and Ethnic Qualifiers in LCSH."
Friday, June 15, 1:00-4:00 pm, Argent Hotel, City.
Instructor: Barbara Conaty. Preregistration only.
RLG RLIN Strategy Focus Group.
Friday, June 15, 2:30-4:30 pm, Marriott-Sierra J.
COLT (Council on Library/Media Technicians) Conference.
Presentation on LC cataloging: Friday, June 15, 3:30-4:20 pm, Holiday Inn (Financial District), speaker Gene Kinnaly.
Quality Books reception in celebration of the CIP programs 30th anniversary.
Friday, June 15, 5:00-7:00 pm, San Francisco Marriott, Salon 4-6, 55 Fourth Street.
This will be an opportunity to thank publishers for their role in the Cataloging in Publication Program. All LC staff attending ALA are invited.
Friday, June 15, 6:00-8:00 pm, Parc Fifty-Five-Da Vinci.
Member from LC: Lynn El-Hoshy. Continues Saturday, June 16.
OLAC (Online Audiovisual Catalogers, Inc.) Cataloging Policy Committee.
Friday, June 15, 7:30-9:30 pm, Argent Hotel-Franciscan III.
Saturday, June 16, 7:00-8:30 am, Argent Hotel-City.
OCLC Forest Press editor-in-chief: Joan S. Mitchell.
Dewey assistant editors: Julianne Beall, Winton Matthews, Gregory New.
ALCTS CCS CC: DA Task Force on Specific Characteristics of Electronic Resources.
Saturday, June 16, 8:30-11:00 am, Hyatt Regency-Garden Room B.
ALCTS Organization and Bylaws Committee.
Saturday, June 16, 8:30 am-12:30 pm, Westin St. Francis-Sussex Room. Continues Tuesday, June 19.
MARBI. Saturday, June 16, 9:30 am-12:30 pm.
LC representative: Sally McCallum; also Rebecca Guenther, Jean Hirons. Meeting continues Sunday, June 17.
ALCTS CCS Policy & Research Committee.
Saturday, June 16, 2:00-4:00 pm, Grand Hyatt-San Francisco B.
ALCTS CCS Committee on Education, Training, and Recruitment to Cataloging.
Saturday, June 16, 2:00-4:00 pm, Stanford Court-Gold Room.
Saturday, June 16, 2:00-5:30 pm, Marriott-Salon 7.
PCC CONSER Publication Pattern Task Force Meeting.
Saturday, June 16, 4:00-6:00 pm, Hilton & Towers-OCLC Red Suite.
Saturday, June 16, 8:00-10:00 pm, Marriott-Laurel.
Sunday, June 17, 8:00-9:30 am, Grand Hyatt-Merced. Co-leader: Jean Hirons.
MAGERT Cataloging and Classification Committee.
Sunday, June 17, 9:30-11:00 am, Marriott-Golden Gate B3.
Sunday, June 17, 9:30 am-12:30 pm, Canterbury Hotel-Garden/Lanai Room. Continues Monday, June 18.
LC liaison: Lynn El-Hoshy. Dewey report: Julianne Beall.
Sunday, June 17, 10:00 am-12:00 pm, Grand Hyatt-San Miguel.
Sunday, June 17, 11:30 am-12:30 pm. Hilton & Towers-Union Square 22.
WebDewey in CORC Focus Group.
Sunday, June 17, 2:00-3:30 pm, San Francisco Hilton & Towers, OCLC Blue Suite.
DDC editors will be present.
LITA/ALCTS ACIG (Authority Control Interest Group in the Online Environment).
Program: "By What Authority? How Multiple Sources of Authority are Changing Our Concept of Control."
Sunday, June 17, 2:00-5:30 pm, Hilton & Towers-Continental Ballroom 7-9.
Speaker on "Authority Control on the Web:" Barbara Tillett.
LC report and incoming ACIG chair: Ann Della Porta.
Sunday, June 17, 2:00-5:30 pm, Canterbury Hotel-English/Garden/Lanai Rooms.
LC representative: Sally McCallum; also Rebecca Guenther. Continued from Saturday, June 16; continues Monday, June 18.
ALCTS CCS Cataloging of Childrens Materials Committee.
Sunday, June 17, 2:00-5:30 pm. Hilton & Towers-Union Square 12.
Sunday, June 17, 4:30-5:30 pm, Cathedral Hill-California Room.
LC/RUSA Forum on Digital Reference and Bibliographic Control: Options for Collaboration.
Sunday, June 17, 4:30-6:30 pm, Grand Hyatt San Francisco, Dolores Room.
Hosted by Beacher Wiggins, Director for Cataloging and Diane Kresh, Director, Public Service Collections.
PCC Continuing Education Sponsors Forum.
Sunday, June 17, 4:30-6:00pm, Grand Hyatt-Sausalito.
PCC Participants Discussion Group Meeting.
Sunday, June 17, 7:00-9:00 pm, Hilton & Towers, Continental Ballroom 1-3.
Also attending from LC: John Byrum, Ana Cristan, John Mitchell, Susan Morris, Beacher Wiggins.
Monday, June 18, 8:00 am-12:30 pm, Cathedral Hill-International Room. Continued from Sunday, June 17.
ALCTS CCS Copy Cataloging Discussion Group.
Monday, June 18, 9:30-11:00 am, Moscone Convention Center-Room 228.
"CIP: a Vision for the Future," sponsored by ALA/ALCTS.
Monday, June 18, 2:00-4:00 pm, Moscone Convention Center, Room 306.
John Celli with Craig Van Dyck, vice-president of Manufacturing, Scientific, Technical, Medical Publishing, John Wiley & Sons, and Pat Thomas, 44-year librarian and Margaret Mann Award recipient.
Includes demo of the New Books Program.
Monday, June 18, 2:00-4:00 pm, Marriott-Salon 10/11.
ALCTS SS Committee to Study Serials Cataloging.
Monday, June 18, 2:00-4:00 pm, Cathedral Hill Hotel-International Room.
LC report, etc: Jean Hirons.
Monday, June 18, 2:00-4:00 pm, Marriott-Golden Gate A3.
PLA Cataloging Needs of Public Libraries Committee.
Monday, June 18,2:00-4:00 pm, Hyatt Regency-Pacific Concourse H/I.
Monday, June 18, 2:00-4:00 pm. Pan Pacific-Olympic C.
LC representative: Sally McCallum; also Rebecca Guenther. Continued from Sunday, June 17.
Tuesday, June 19, 8:30am-12:30 pm, Moscone Convention Center-Room 226. Continued from Saturday, June 16.