text:
\section{Introduction}
With the availability of very high energy jets in heavy-ion collisions at the Large Hadron Collider (LHC)~\cite{Appelshauser:2011ds,Cole:2011zz,Tonjes:2011zz}, the study of jet modification
has moved far beyond the suppression of leading hadrons. In order to theoretically calculate the large number of new measurements
such as multi-particle correlations, jet shapes, flow of energy-momentum in and out of jet cones etc., one requires a Monte-Carlo
based event generator. Even reconstructed single particle observables such as the fragmentation function of the remnant
jets as measured by the CMS and ATLAS collaborations~\cite{Chatrchyan:2012gw,ATLAS:2012ina} are, in principle, multi-particle
effects, where the jet has to be reconstructed to some extent, from the parton shower. A proper description of all such processes requires a
Monte-Carlo event generator.

Monte-Carlo based event generators represent one of the most important interfaces between theory and experiment
 in high energy processes, especially those involving QCD jets. In vacuum these are very well
 developed~\cite{Bengtsson:1987kr,Marchesini:1991ch,Gleisberg:2008ta}. So far the development of jet modification
 in the presence of a medium has been somewhat varied. This is mostly due to the lack of consensus on the right
 analytic approach to jet modification. Prior to the commissioning of the LHC, there existed four different analytical energy loss
 approaches~\cite{Gyulassy:2000fs,Wiedemann:2000za,Guo:2000nz,Arnold:2002ja} which were equally successful at describing
 high transverse momentum (high $p_{T}$) hadron suppression data from the Relativistic Heavy-Ion Collider (RHIC).
 All of these were based on perturbative QCD (pQCD).

 Two of these analytical calculations, enhanced with the inclusion of dynamical media,
 the Armesto-Salgado-Wiedemann (ASW) scheme~\cite{Armesto:2003jh} and the Arnold-Moore-Yaffe (AMY) scheme~\cite{Qin:2007rn} have been incorporated within Monte-Carlo event generators. The ASW scheme has been incorporated within  Q-PYTHIA~\cite{Armesto:2009fj}, while the AMY scheme has been incorporated
 within the MARTINI Monte-Carlo event generator~\cite{Schenke:2009gb}.
 Along with these, there are also the first principles event generators: JEWEL~\cite{Zapp:2008gi,Zapp:2012ak} and
 YaJEM~\cite{Renk:2009hv,Renk:2012ve}, which are not completely based on any of the analytical models, and incorporate
 medium effects within vacuum parton showers by modifying various matrix elements by hand.
 This was also the methodology followed by the very first jet modification event generator PYQUEN~\cite{Lokhtin:2005px}, where the
 energy loss kernel was loosely based on the Baier-Dokshitzer-Mueller-Peigne-Schiff (BDMPS) approach~\cite{Baier:1996sk}.

 The generic methodology in all these cases has been to take the standard vacuum event generator and either add a component that represents medium
 effects, after the full vacuum shower has been generated, or to enhance the vacuum shower algorithm itself such that the resulting shower is modified, i.e.,
 vacuum and medium induced radiation is accounted for simultaneously.
 Besides the variety of technical issues that must be surmounted in the construction of an in-medium jet Monte-Carlo event generator, two fundamental
 problems need to be dealt with, which have no analog in vacuum: The introduction of space-time structure (and fluctuations in space-time structure)
 in the shower, and a mechanism of hadronization where partons from the hot dense medium will coalesce with partons from the jet to form hadrons.
 None of the of the above mentioned schemes addresses either of these two effects in a satisfactory manner.

 In this paper, we attempt to solve the first of these problems: the incorporation of a theoretically consistent space-time structure, as well as fluctuations in
 space-time structure,\footnote{Note: fluctuations in space-time structure have been phenomenologically introduced in YaJEM~\cite{Renk:2009nz}.} within the event generator framework. The Monte-Carlo event generator will be based on the Higher-Twist scheme, and this
 paper will contain the first set of results within such a framework. The event generator will be referred to as the
 Modular-All-Twist-Transverse-and-Elastic-scattering-induced-Radiation (MATTER++) event generator. The `++' simply indicates the choice of programming language.
 The remaining terms in the moniker refer to the underlying theory which may be found in Refs.~\cite{Majumder:2008zg,Majumder:2009ge}.

 The remaining paper will be organized as follows: Sec.~II will contain a terse review of final state event generation for jets in vacuum. Sec.~III will discuss
 how the light-cone location of a split, which is normally integrated out, may be reintroduced into the calculation of jet modification. In Sec.~IV, we will outline the
 basic components of our Higher-Twist based event generator. In Sec.~V, we will present results of our numerical calculations of jet modification in a static
 medium of finite length. Concluding discussions are presented in Sec.~VI.

 \section{Final state Vacuum event generation}

 In this section we will review the simulation of parton showers in vacuum.
In order to illustrate the reintroduction of space-time in jet shower development, we
will set up the process within the framework of Deep-Inelastic Scattering (DIS). We will take a factorized approach,
valid at high energies, in the presence of a hard scale.
We will ignore the development of the initial state space-like shower and
only consider the final state time-like shower.

A hard lepton with incoming
momentum $L_{i}$  scatters off a proton with incoming momentum $P$ and exits with an outgoing momentum $L$.
The proton is shattered into a large number of final hadronic states. The
inclusive differential cross-section for an arbitrary process with hadrons with momenta $p_{1} \ldots p_{N}$, in the single photon approximation, may be expressed as,
\bea
\frac{ d \sigma  }{ d^{3} L d^{3} p_{1} \cdots d^{3} p_{N}   } = \frac{\A_{\rm EM}^{2}}{2 \pi s E_{L} Q^{4}} \mathcal{L}^{ \mu \nu }
\frac{ d W_{\mu \nu} }{ d^{3}  p_{1} \cdots d^{3} p_{N} } ,
\eea
where, $\mathcal{L}^{\mu \nu} $ is the leptonic tensor, all factors which represent the interaction of the incoming and outgoing lepton with the exchanged photon are contained within $\mathcal{L}^{\mu \nu}$. The hadronic tensor $W^{\mu \nu}$ contains the entire set of
hadronic interactions including the interaction of the proton with the photon. The Mandelstam variable $s = (x_{B} P + q )^{2}$.
The Bjorken variable $x_{B} =  Q^{2}/(2 P \x q )$.
We choose a frame where the momentum of the photon is
given in light-cone coordinates as,
\bea
q \equiv \left[  \frac{Q}{\sqrt{2}}, - \frac{Q}{\sqrt{2}}, 0,0 \right],
\eea
 often referred to as the Breit frame.

The simplest instance of a hadronic final state is a single quark in the final state. In this case the
hadronic tensor has a simple factorized form,
\bea
{W_0}^{\mu \nu}
&=&  \frac{2 \pi x_B}{2 Q^2} \tr \left[ \f{P} \g^\mu \left( \f{q} + x_B \f{P} \right) \g^\nu  \right]
\sum_q Q_q^2f_q (x_B)  \nn \\
&=& 2 \pi  [ g^{\mu -} g^{\nu +} + g^{\mu +} g^{\nu -} - g^{\mu \nu} ]  \sum_q Q_q^2 \ \\
\ata \int \frac{d y^-}{2\pi} e^{-ix_B P^+ y^-} \hf \lc P | \psibar(y^-) \g^+ \psi(0) | P \rc \nn.
\eea
 In the equation above, $Q_{q}$ represents the charge of the quark in units of the electron's charge, $f_{q}$  represents the
 light-cone distributions of quarks inside the proton.

 The equation above is the integral hadronic tensor. The differential
 hadronic tensor as a function of the three dimensional momentum of the outgoing quark is given as,
\bea
\frac{d^3 W_0^{\mu \nu}}{d^3 l } =  W_0^{\mu \nu} \kd^2 (\vec{l}_\perp  )\kd( l^{-} - q^{-} ), \label{d_W_0}
\eea
where, the outgoing quark carries the \nolinebreak{($-$)-lightcone} momentum of the incident photon.
The equation above represents a simple expression, where the production cross section of the hard parton, contained within $W_{0}^{\mu \nu}$,
is factorized from the final state distribution, which in this case is simply the three dimensional delta function $\kd^{3}(\vec{l} - \vec{q})$.
In what follows, we will not discuss the production process of the hard parton and only focus on the final state propagation.
In the case of a parton produced close to its mass shell, there is scarce little beyond the 3-D delta function, that may be calculated with
pQCD.

For the case of hard parton, produced off its mass shell (time like for a final state parton), one has to include multiple final state emissions.
In this process of emission, the virtuality of the hard parton is gradually reduced to a low enough scale where hadronization can begin to set in.
While the hadronization process requires phenomenological modeling, emissions which lead to the reduction of the virtuality from $Q^{2}$ to a
minimum hard scale where pQCD is applicable can be described by constructing and simulating a Sudakov form factor. For the case of a quark
in vacuum, the Sudakov form factor is given as,
\bea
S(Q_{0}^{2},Q^{2}) = \exp\left[ - \!\!\!\int\limits_{2 Q_{0}^{2}}^{Q^{2}}\!\! \frac{d\mu^{2}}{\mu^{2}} \frac{\A_{S}(\mu^{2})}{2 \pi}
\!\!\! \int\limits_{Q_{0}/Q}^{1-Q_{0}/Q} \!\!\!\!\!\!\!dy  P_{qg}(y) \right]\!. \label{vac-sud}
\eea
In the equation above, $P_{qg}(y)$ is the usual LO splitting function for a quark to radiate a gluon which carries a forward
momentum  of $(1-y)q^{-}$, and have its light-cone momentum degraded to $yq^{-}$~\cite{Altarelli:1977zs}. The quantity $\mu^{2}$ represents
the highest allowed virtuality of the parton undergoing the split and is also the running scale in the process. The Sudakov form factor represents
the probability that there is no emission, between the scales $Q_{0}^{2}$ to $Q^{2}$.

The procedure to generate a shower in vacuum is now completely straightforward, and has been described in several texts~\cite{Ellis:1991qj}.
One samples the Sudakov form factor and obtains the highest virtuality that the remaining process may possess. This is followed by
sampling the splitting function, to obtain a fraction $y$ which represents the fraction of light-cone momentum left in one of the partons after the
split. This process is then iterated for each virtual parton to generate the full shower. The cascading process in any part of the shower is stopped when the virtuality of that part reaches $Q_{0}^{2}$.

In the process of shower development in the vacuum, the entire cascade process may be carried out in momentum space.
Note that space-time does not enter in the formulation of the Sudakov form factor in vacuum [Eq.~\eqref{vac-sud}].
In what follows, we will consider the modification of this process in the presence of a medium; here the location of a
hard parton will need to be retained at all stages of the calculation. The modification of the shower Monte-Carlo algorithm will be
discussed in Sect.~IV.

 \section{The re-introduction of space-time in Monte-Carlo event generation}

In the preceding section, the pQCD based vacuum shower Monte-Carlo formalism was reviewed. In this well tested set up, no information about the
space-time location of the shower is retained. In this section we will make the most minimal modification to the formalism to include this information.
In the subsequent section, we will describe the modification to the propagation of non-emitting partons, and that to the Sudakov
form factor due to scattering in the medium.

Consider, for simplicity, the process of high energy DIS with a near on-shell quark, scattering off the gluon field generated in a medium.
In this limit, the multiple scattering expression, for a quark propagating through the medium without emission, can be expressed using
almost classical arguments as the gradual linear broadening with distance travelled. At some point in its path, the quark will radiate a
gluon and these two partons will, beyond the formation length, propagate as independent particles multiply scattering off the gluon
field. At the split, the two partons will separate from each other with a large and opposing transverse momenta $l_{\perp}$. The
accrued transverse momentum $k_{\perp}$  adds incoherently to this large momentum $l_{\perp}$.

To carry out the program of broadening described above, the crucial piece of information required is the (light-cone) location, beyond which the
two partons that have split from the parent parton, may be considered to scatter independently.
The reader will note that while the location of a split, on average, will be different between jets in vacuum versus those in medium, this
remains a well defined question even for the case of jets in vacuum.
We will first attempt to answer the question of the location of splits for
jets in vacuum.

\begin{figure}[htbp]
\resizebox{3in}{2.5in}{\includegraphics{gluon_emit_no_scat_W_mu_nu_lables}}
    \caption{ The diagram for the hadronic tensor of DIS on a proton with an outgoing quark and a radiated gluon.}
    \label{fig1}
\end{figure}

Consider the process of semi-inclusive DIS on a proton, with a hard quark and a radiated gluon in the final state (illustrated in Fig.~\ref{fig1}). The hadronic
tensor may be expressed as,
\bea
{W_0}^{\mu \nu}
&=&  \int d^4y_0 \lc P |  \psibar(y_0) \g^\mu  \widehat{\Op} \g^\nu \psi(0) | P \rc  \nn \\
&=& \int d^4 y_0\tr [\frac{\g^-}{2} \g^\mu \frac{\g^+}{2} \g^\nu ] F(y_0) \Op(y_0) . \label{gen-struct}
\eea
The location of the quark in the complex conjugate is $y_{0}$ and its location in the amplitude is
set as the origin. The factor $F(y_{0})$ represent the expectation of operators that constitute the initial
state, while $\Op(y_{0})$ constitutes the expectation of operators in the final state.

In DIS, the momentum components of the hard photon $q^{-}$ and $q^{+} = Q^{2}/(2 q^{-})$ are experimental
measurements. In most analytical calculations, any uncertainty in these quantities is averaged over.
Since, no attempt to determine the space-time location of the hard scattering is made, the uncertainty in these
quantities is minimal. However, this is not the case for $p_{0}^{+} = x_{B} P^{+}$. The value of $x_{B}$ is an approximate
average value. Hard quark jets are produced far off their mass shell. The cause of this off-shellness is the
uncertainty in $p_{0}^{+}$. The formation length of any emission in the jet's shower development depends on the virtuality of the
emitting parton; more precisely, it depends on the uncertainty in the virtuality, limited by the virtuality itself.
To elucidate the
space-time structure of the jet created by this hard interaction, the uncertainty in the various momentum components
has to be taken into account.

No doubt, all other energy-momentum and space-time factors will exhibit uncertainties. However, as $p_{0}^{+}$ represents the largest
scale in the problem, the uncertainty in this quantity has the maximal effect on the space time structure of the developing jet.
Let us denote the momentum of the final state quark as $p \equiv [p^{+},p^{-},p_{\perp}]$.
Quark jets produced in DIS have a large $(-)$-light-cone momentum component and a small $(+)$-component.
As a result, the
space-time profile of the jet is concentrated near the $x^{+} = 0$ light-cone. In this first attempt, we will not probe the
deviation of the jet away from the strict light-cone. As a result, we will ignore the uncertainty in $p^{-}$ (or $p_{\perp}$)
and only focus on the uncertainly in $p^{+}$. Note that the uncertainty in $p_{0}^{+}$ directly translates into an uncertainty in $p^{+}$.
In a future effort both uncertainties will have to be considered. An uncertainty in $p$ is most straightforwardly introduced by setting the $p_{0}$ vector
to be different in the amplitude and complex conjugate. In the end, the offset in all components of $p$ except in $p^{+}$ will be ignored.

In the presence of this uncertainty in $p$, the initial state operator expectation $F(y_{0})$ is unchanged:
\bea
F(y_0) = \lc P | \psibar(y_0) \frac{\g^+}{2} \psi(0) | P \rc , \label{F(y_0)}.
\eea
The final state operator expectation becomes
\bea
\Op &=& \tr \left[ \frac{\g^-}{2} \widehat{\Op} \right]  \label{O_1}\\
 &= & \int \frac{d^4 l}{(2\pi)^4}   d^4 z d^4 {z\p}
\frac{d^4 l_q}{(2\pi)^4}\frac{d^4 p_0}{(2\pi)^4} \frac{d^4 {p\p}_{0}}{(2\pi)^4}\nn \\
\ata   \tr \left[  \frac{\g^-}{2} \frac{-i (\f p_0 + \f q )}{ (p_0 + q )^2 - i \e }
i\g^\A  \f l_q   2\pi \kd (l_q^2)  \right.  \nn \\
\ata \left. G_{\A \B} (l)   2\pi \kd (l^2)  (-i\g^{\B})
\frac{ i (\f p_0\p + \f q )}{ (p_0\p + q )^2 +  i \e }  \right] \nn \\
\ata e^{i q \x y_0 }e^{ -i (p_0 + q) \x ( y_0 - z) }
e^{-i l \x (z - z\p)} e^{-i l_q \x (z - z\p)} \nn \\
\ata e^{ -i (p_0\p + q) \x z\p  } g^2  . \nn
\eea
As pointed out in the diagram in Fig.~\ref{fig1}, the incoming quark momentum in the amplitude and
complex conjugate ($p\p_{0}$ and $p_{0}$) are mismatched. Similarly, the location of the emission of the
gluon is denoted as $z\p$ in the amplitude and $z$ in the complex conjugate. Note that they do not have to be
at the same point.

The phase factors and the $z , z\p$ integration may be simplified as follows,
\bea
\Gamma = \int  d^{4} \bar{z} d^{4} \D z e^{ ( \bar{p}_{0} + \bar{q} - l - l_{q} )\x( \D z )  }  e^{  i (\D p_{0}  )\x \bar{z} }.
\eea
In the equation above, $\bar{p}_{0} = (p_{0} + p\p_{0})/2$ and $\D p_{0} = p_{0} - p\p_{0}$.
Similarly the
two positions are defined as $\bar{z} = (z + z\p)/2$ and $\D z  = z - z\p$.
Carrying out the $\D z^{-}$  integral we obtain the usual relation that $\bar{p}^{\,+} + \bar{q}^{\, +} = l^{+} + l_{q}^{+}$.

In the limit that $p_{0}^{-}$ and ${p\p}_{0}^{-}$ are vanishingly small, the
matrix element may be simplified as,
\bea
\Op  &= & \int \frac{d^2 l_{\perp} dl^{-} }{(2\pi)^3}   d \bar{z}^{-} d^{2} \bar{z}_{\perp}
\frac{d \D p_0^{+}  d^{2} \D { p_{0} }_{\perp} }{(2\pi)^{3}}  \frac{ d^{2} { \bar{p}_{0} }\mbx_{\perp} }{ (2 \pi)^{2} } \nn \\
\ata  g^2  \tr \left[  \frac{\g^-}{2} \frac{-i (\f l+ \f l_{q} )}{ (l + l_{q} )^2  }
i\g^\A  \f l_q   G_{\A \B} (l)  (-i\g^{\B}) \right.  \nn \\
\ata \left.
\frac{ i (\f l + \f l_{q} )}{ ( l + l_{q}  )^2  }  \right] e^{-i [ ( x_{B} + x_{L} ) p^{+} \D y_{0}^{-} -  { \bar{p}_{0} }\mbx_{\perp} \x \D { y_{0} }\mbx_{\perp} ]}\nn \\
\ata   e^{- i ( \D p_{0}^{+} \bar{y}_0^{-}  - \D {p_{0}}_{\perp} \x \bar{y}_{\perp} ) }
e^{  i ( \D p_{0}^{+} \bar{z}^{-} - \D { p_{0} }_{\perp} \x \bar{z}_{\perp} ) }   .
\eea
In the equation above, $p^{0} y^{0}$ is expressed as $ \D p^{0} \bar{y}_{0} + \bar{p}_{0} \D y_{0} $.
Since no part of Eq.~\eqref{O_1} depends on $p^{-}_{0}$
or ${p\p_{0}}^{-}$, these have been integrated out to obtain $\kd (z^{+})  \kd ({z\p}^{+})$,
localizing the process on the light cone. Note, this would be modified if $\D q^{-}$ had been retained.
This leaves the transverse momentum integrals. Carrying out the $\bar{z}_{\perp}$ integrals, sets $ {p_{0} }_{\perp} = { p'_{0} }_{\perp} $.
One may also integrate out the $\D {p_{0}}_{\perp}$ which yields a $\kd$-function, that may be used to set $\bar{z}_{\perp} = { \bar{y}_{0}  }\mbx_{\perp}$.

The final integration that is left is that over $\bar{z}^{\,-}$. In order to carry it out, one needs to evaluate the $\D p_{0}^{+}$ distribution.
To compute this exactly, one has to carry out the integral,
\bea
&&\int d \bar{y}_{0} e^{ - i  \D p_{0}^{+} \bar{y}_{0}^{-} }  \\
\ata \left\lc P \left| \psibar\left( \bar{y_{0}}^{ -} + \frac{\D y^{-}}{2} \right) \g^{+} \psi \left( \bar{y}_{0}^{- } - \frac{\D y^{-}}{2} \right) \right| P \right\rc .\nn
\eea
Note that in Eq.~\eqref{gen-struct}, there is no integration over the mean distance $\bar{y}_{0}$. This is because, we have set the location of the
scattering in the amplitude to be the origin. But in reality, all locations in the nucleon are not equivalent and one should average over this variable.
The result of such an averaging may be expressed as the usual parton distribution function for $\bar{p}_{0}^{+}$ times a distribution for
the offset $\D p_{0}^{+}$.
For this first attempt, we will assume a Gaussian uncertainty for the $\D p^{+}_{0}$ distribution:
\bea
\rho(\D p_{0}^{+}) = \frac{e^{ - \frac{{\D p_{0}^{+}}^{2}}{2\sigma^{2}} }}{\sqrt{ 2 \pi \sigma^{2} }}. \label{drho-dist}
\eea
The width depends on the scale of the process ($Q^{2}$): Processes with higher $Q^{2}$ or rather higher $q^{+}$ have larger widths.
We will set the width using a bootstrap method where, given a width,  we first calculate the distribution of locations $\bar{z}^{-}$  where the
split occurs, and then average over these locations to obtain the mean distance of the split. The distribution of $\bar{z}^{-}$ is obtained by
Fourier transforming the distribution for $\D p^{+}$, which will also yield a Gaussian distribution for $\bar{z}^{-}$
(Note: the distribution of $\D p^{+}$ is identical to the distribution of $\D p_{0}^{+}$).
The width is then dialed so that this mean distance equals the formation time for a given $q^{-}$ and $Q^{2}$.

As a result of these simplifications, the produced off-shell quark has a momentum of $p \equiv [p^{-},p^{+},0,0] $.
We obtain the forward light-cone momentum $p^{-} = q^{-}$ and a virtuality $\mu^{2} = 2 p^{+} p^{-} = 2 p_{0}^{+} q^{-}$,
where $p_{0}$ is the momentum of the incoming quark.
The gluon radiated from this quark will have a light-cone formation time (equal to the light-cone formation length for a hard parton),
\bea
\tau_{f}^{-} = \frac{ 2 p^{-} }{\mu^{2}}  = \frac{2 }{ p_{0}^{+} }. \label{tau}
\eea
Thus, the $\D p_{0}$ distribution will have a width of $\sigma = 2 p^{+} / \pi = 2 p_{0}^{+}/\pi$. This will ensure that on integrating the Gaussian distribution
from a distance $\bar{z}^{\, -} =0 $ to $\infty$, the mean light-cone distance will be equal to the light-cone formation time in Eq.~\eqref{tau}.
To obtain a distribution of formation times, we simply have to sample this Gaussian distribution for positive values of the light-cone location of
the split.

While motivated for the case of the first emission in DIS, the set up may be used for the case of multiple emission: One simply determines the
large light-cone momentum $p^{-}$ and the off-shellness $\mu^{2}$, or rather the smaller light-cone momentum $p^{+} = \mu^{2}/(2p^{-})$, and then computes the formation time. Assuming that the uncertainly in $p^{+}$ is of the order of (but smaller than) $p^{+}$ itself, we obtain a distribution in
formation times by Fourier transforming Eq.~\eqref{drho-dist},
\bea
\rho(x^{-} ) = \sqrt{ 2 \pi \sigma^{2} }e^{- \frac{\sigma^{2} {x^{-}}^{2}}{2} }, \label{x-dist}
\eea
with $\sigma = \sqrt{2} p^{+} /\sqrt{\pi}$.
The inclusion of this distribution in $x^{-}$, in combination with the distribution in $\bar{p}^{+}$ which will be obtained by sampling the Sudakov form factor
convert the shower formalism into a Wigner Transform like formalism where the two non-conjugate components of space-time and momentum are retained.
These will be used to determine the location of the split of a particular parton.

In the set up described above, to obtain a particular splitting length, one needs to know the two components $p^{-}$ and $p^{+}$. In the
subsequent section we will describe how to obtain these momentum components $p^{-}$ and $p^{+}$ from the calculation of the
Sudakov form factor. The Sudakov form factor will be determined for the case in vacuum and in the case of a medium. The effect of the medium
will enter only in the determination of the distribution of $p^{+}$ and $p^{-}$. Once $p^{+}$ and $p^{-}$ have been determined, the distribution in
Eq.~\eqref{x-dist} can be used to find the splitting distance for a particular event.

 \section{Final state In-Medium event generation}

 In the preceding section, the means to calculate the distribution of splitting lengths was outlined.
 We have refrained from denoting the lengths obtained from sampling Eq.~\eqref{x-dist} as formation
 lengths (or formation times). The mean of the splitting lengths will be denoted as the formation length (or formation time).
 In the calculation of the distribution of splitting lengths, the input is composed of the light-cone momentum components
 of the hard parton which will undergo the split. In this section we will outline how these components are determined.

 We return to the case of a hard quark produced in DIS on a nucleon, and simply replace the nucleon with a large
 nucleus. The photon hits a quark in one of the nucleons and then sends it back through the nucleus where its
 evolution to a jet is modified by the presence of a nuclear medium. One may divide the modification into two
 parts, one which modifies the transverse momentum distribution of a propagating parton without inducing it to
 radiate and another which changes the radiation probability of the virtual parton. As in the case of the
 analytic calculation~\cite{Majumder:2007hx,Majumder:2009ge}, we will compute these separately and then incorporate these
 within one calculation.

 The modification of the transverse momentum distribution, of the outgoing quark, without emission, in a medium, is trivial:
 As pointed out in~\cite{Majumder:2007hx,Majumder:2008zg,Qin:2012cz}, this may be
 easily expressed by simply replacing the $\kd$-function by position dependent Gaussians. In this first
 attempt to convert the Higher-Twist approach to a Monte-Carlo, we will ignore elastic drag.

In the following, the production of the hard parton will no longer be considered and the focus will lie solely on the fate of the final state parton.
Transverse momentum broadening is achieved by sampling a unitary Gaussian distribution.
The parton enters the medium with a narrow distribution in transverse momentum [$\kd(\vec{l}_{\perp})$], which is then broadened to a
two dimensional unitary Gaussian distribution, whose width depends on the length traversed by the parton,
\bea
\kd(\vec{l}_{\perp}) \ra \phi(L^-,\vec{l}_\perp) = \frac{1}{4 \pi D L^-} \exp \left\{-  \frac{l_\perp^2}{4 D L^-} \right\}. \label{solution}
\eea
In the equation above, $D$ is the transverse momentum diffusion coefficient, the well known transport coefficient $\hat{q} = 4 D$. The light
cone length $L^{-}$ is the light-cone length traversed in their medium. In the case that the medium is not uniform,
one may simply replace $DL^{-} \ra \int d L^{-} D (L^{-})$.

To determine the lengths traversed in the medium, one requires the locations of the the various splits that a jet undergoes as it
propagates through the medium. To be specific, let us consider a single hard quark propagating through a dense medium undergoing multiple
hard scattering, and both vacuum and medium induced radiation.
As mentioned in the preceding section, to determine the location of the splits, one needs the
two light-cone components of the virtual quark. The ($-$)-component $p^{-}$ will be considered to be large and the $(+)$-component
$p^{+}$ will be considered to be small (but still much larger than $\Lambda_{QCD}$). The virtuality $Q^{2} = 2 p^{+} p^{-}$.

In order to obtain the distribution of leading hadrons emanating from the fragmentation of this hard quark, one would compute the medium
modified fragmentation function~\cite{Majumder:2009zu}. This requires the solution of the
Dokshitzer-Gribov-Lipatov-Altarelli-Parisi (DGLAP) evolution equation~\cite{Dokshitzer:1977sg,Gribov:1972ri,Gribov:1972rt,Altarelli:1977zs} in the presence of a medium~\cite{Majumder:2009zu},
\bea
\mbx\!\!\!\!\!&& \frac{\prt {D_q^h}(z,Q^2\!\!,p^-)|_{\zeta_i}^{\zeta_f}}{\prt \log(Q^2)} = \frac{\A_s}{2\pi} \int\limits_z^1 \frac{dy}{y}
P(y) \nn \\
\mbx\!\!\!\!\! \ata \left[ {D_q^h}\left. \left(\frac{z}{y},Q^2\!\!,p^-y\right) \right|_{\zeta_{i}}^{\zeta_f}  \right. \nn \\
\mbx\!\!\!\!\! &+&  \int\limits_{\zeta_i}^{\zeta_f} d\zeta  \left.K_{p^-,Q^2} ( y,\zeta)  {D_q^h}\left. \left(\frac{z}{y},Q^2\!\!,p^-y\right) \right|_{\zeta}^{\zeta_f} \right] .  \label{in_medium_evol_eqn}
\eea
In the equation above ${D_q^h}(z,Q^2\!\!,p^-)|_{\zeta_i}^{\zeta_f}$ is the medium modified fragmentation function for a hadron to
to fragment with light-cone momentum $zp^{-}$ ($0<z<1$), from a hard
quark with a light-cone momentum $p^{-}$, and virtuality $Q^{2}$.
For this fragmentation function, the quark commences propagation at $\zeta_{i}$ and
exits at $\zeta_{f}$. The factor $P(y)$ represents the un-renormalized splitting function, and $y$ represents the
fraction of momentum which remains in the quark after a gluon has been radiated.
The leading twist contribution to the multiple scattering, single emission kernel $K$, is given as
\bea
K_{p^-,Q^2} ( y,\zeta) = \frac{2 \hat{q} }{Q^{2}}
\left[ 2 - 2 \cos\left\{ \frac{Q^2 (\zeta - \zeta_i)}{ 2 p^- y (1- y)} \right\}  \right] . \label{kernel}
\eea
The full evolution equation for the medium modified fragmentation functions will include
contributions from gluon fragmentation
functions which have a similar in-medium evolution.

 We should point out at this stage, that in the Higher-Twist approach, multiple emissions are ordered in transverse momentum as they are in
 vacuum DGLAP emission. Multiple scattering is suppressed by powers of the hard scale and enhanced by the length of the medium traversed by a parton.
Such ordered multiple emission in the presence of multiple scattering is only considered when $\hat{q}L \ll Q^{2}$ ($L$ is the length traversed by parton
before splitting) i.e., when the multiple soft scattering
does not produce a considerable affect on the transverse momentum distribution between the partons post split (or the virtuality distribution of the
parent parton). Once $Q^{2}$ becomes too small, Higher-Twist based calculations have to be abandoned. We should point out that beyond this
limit, the ordering of multiple emissions is, as yet, unsettled~\cite{CasalderreySolana:2012ef}.

Since the medium modified evolution equations are valid in a similar range of momenta as the vacuum emission process, we may set up a Sudakov
form factor for the Higher-Twist based multiple scattering induced emission process. In this case, the medium modified Sudakov form factor for a quark with light-cone momentum $p^{-}$, with a maximum virtuality $Q^{2}$, propagating through a dense medium, starting at the light-cone location $\zeta_{i}^{-} $ is given as,
\bea
\mbx\!\!\!\!&& S_{\zeta_{i}^{-}}(Q_{0}^{2},Q^{2}) = \exp\left[ - \int\limits_{2 Q_{0}^{2}}^{Q^{2}} \frac{d\mu^{2}}{\mu^{2}} \frac{\A_{S}(\mu^{2})}{2 \pi}  \right.
\label{in-med-sud} \\
 \mbx\!\!\!\! \ata \left. \int\limits_{Q_{0}/Q}^{1-Q_{0}/Q} \!\!\!\!\!dy  P_{qg}(y)
 %
 \left\{  1 + \int_{\zeta_{i}^{-}}^{\zeta_{i}^{-} + \tau^{-}} \!\!\!\!\!d \zeta K_{p^-,Q^2} ( y,\zeta) \right\} \right] . \nn
\eea
In the equation above, the vacuum portion of the argument of the exponent is identical to Eq.~\eqref{vac-sud}. The medium portion is
integrated from the location $\zeta_{i}^{-}$ to the location $\zeta_{i}^{-} + \tau^{-}$. The choice of the distance $\tau$ is significant.
There are two ways to deal with this: One method is the use the sampled value of $Q^{2}$ and the known value of forward light-cone
momentum $p^{-}$ (which is equal to $q^{-}$ in this case) and substitute $p^{+} = Q^{2}/(2p^{-})$ in Eq.~\eqref{x-dist}. One can then
sample this distribution and obtain a particular splitting length $x^{-}$. This length may then be substituted in Eq.~\eqref{in-med-sud}
to compute the Sudakov factor. The downside of this method is that one will always get a random length $x^{-}$ for a given step
in the Monte-Carlo simulation [averaging over many such samplings of Eq.~\eqref{x-dist} will yield the mean formation lenght]. As a result
the Sudakov from factor will not be a monotonic function of $Q^{2}$ which will obviously slow down the computational speed of any such
calculation.

An alternative is to use a mean length, which in this case would be the formation length $\tau_{f}^{-}$ based on $p^{-} $ and the chosen virtuality $Q^{2}$.
One may be critical about this mean choice, especially since one is using the mean of the vacuum distribution of splitting lengths as the length of the
medium modified part of the calculation as well. However, this choice of $\tau^{-} = \tau^{-}_{f}$ may also be justified based on the medium
modified calculation. In Fig.~\ref{fig2}, we plot the medium modified single emission kernel. The red solid line is a plot of $K$ from Eq.~\eqref{kernel},
modulo the constant factors $2 \hat{q}/Q^{2}$, as a function of light-cone length $x^{-}$ (in units of the light-cone formation length $\tau_{f}^{-}$).
This is referred to as the GW line as it was first derived for the case of single scattering induced radiation by Guo and Wang~\cite{Guo:2000nz,Wang:2001ifa}.

\begin{figure}[htbp]
\resizebox{2.75in}{2.75in}{\includegraphics{K-plots-cp}}
    \caption{ A comparison between the behavior of the Guo-Wang (GW) and the Aurenche-Zakharov-Zaraket (AZZ) radiation
    kernels as a function of length traversed by parton in a medium.}
    \label{fig2}
\end{figure}

The GW formula has been derived for the case of short lengths in the medium and has the property of continuously growing with distance.
One obtains this formula by ignoring a series of phase factors which are small for short distances~\cite{Wang:2008ti}. However, the GW formula
yields no obvious point to stop the length integration. This is resolved by using the formula derived by Aurenche-Zakharov-Zaraket~\cite{Aurenche:2008hm,Aurenche:2008mq} (referred to
as AZZ and plotted as the dotted line in Fig.~\ref{fig2}).
This formula contains all the phase factors that were ignored by Guo and Wang. It matches with the results of GW for distances
up to the formation length. Beyond the formation length, it deviates from the GW results, turns over and starts dropping down to zero. Beyond twice
the formation length, the AZZ result becomes negative and then oscillates continuously up to infinity.
The interpretation of this result, is that the single emission formula (or perturbation theory up to this order)
is only valid up to a distance of the order of the formation length. Beyond this length, one must use multiple
emissions. Based on these considerations, we chose $\tau^{-} = \tau_{f}^{-}$  and the GW formula for the kernel in Eq.~\eqref{in-med-sud}.
One may also chose $\tau^{-} = 2 \tau_{f}^{-}$ and the AZZ formula to
retain the full range of positive AZZ contributions. For a static homogeneous medium this can be easily equated with the previous prescription by
rescaling $\hat{q}$.

With the Sudakov factor, now completely defined, it may be sampled to obtain the virtuality of a particular parton. The large light-cone momentum
$p^{-}$ and the virtuality $Q^{2}$ can now be used to sample the splitting length distribution in Eq.~\eqref{x-dist} to obtain an event-by-event distance where the
parton will undergo a split. The remaining steps are identical to those in vacuum: one computes the splitting fraction $y$ by sampling the splitting function.
This gives two partons with light-cone momentum $yp^{-}$ and $(1-y)p^{-}$, and transverse momentum $l_{\perp}$ and $-\l_{\perp}$; where
$l_{\perp} = Q^{2}y(1-y)$. The maximal virtuality of the two produced partons is $Q^{2}$; the actual virtuality will be obtained by again sampling the
Sudakov factor for each of these separately.

With the setup described above, we can now generate a parton shower. With the knowledge of the location of the splits, the distance traveled by a
parton between splits is known. This allows for a calculation of the transverse broadening by scattering to be carried out using Eq.~\eqref{solution}.
In the subsequent sections, we will present simple numerical calculations of jet modification in a dense extended medium.

\section{Numerical Simulations}

In the preceding sections, the formalism to carry out event generation of a parton shower propagating through the medium in MATTER++ was set up. In this
section, simple numerical simulations will be presented. In order to study the various facets of jet propagation in a dense medium, independent
from the evolution of the medium itself, in this first effort, we will only consider jet propagation in a finite sized static medium held at a fixed temperature.
This set up is often referred to as the brick~\cite{Armesto:2011ht}. Event generation has been studied within a brick format by several other
authors~\cite{Zapp:2008gi,ColemanSmith:2011rw}. In the remainder of this section, we outline 3 separate calculations: The calculation of the distribution of
surviving quarks and gluons emanating from a single hard quark or gluon, the medium modified fragmentation function, and a medium modified fragmentation
function based on the surviving energy of a hard jet (motivated by recent CMS and ATLAS results).

\begin{figure}[htbp]
\resizebox{3in}{3in}{\includegraphics{q-100-Q-50-vac}}
    \caption{ (Color online) A comparison between the vacuum MC calculation and a DGLAP calculation of the distribution of partons with $Q=1$~GeV, as
    a function of the light-cone momentum fraction $z$. The originating parton is a 100 GeV quark. MC results
    are for 100,000 events. See text for details.}
    \label{fig3}
\end{figure}

The first test of our new Monte-Carlo (MC) formalism will be a comparison of the distribution of partons (with a minimal virtuality of $Q_{0} = 1$~GeV),
 as a function of the longitudinal light-cone fraction $z=p_{h}^{-}/p^{-}$, in the vacuum with standard analytic calculations. In Fig.~\ref{fig3}, we consider
the case of a hard quark with an initial $q^{-}= 100$~GeV and a maximal virtuality of $Q = 50$~GeV. This leads to a shower of partons in the vacuum. The
virtuality drops with each step of the shower until a parton reaches $Q=1$~GeV. The parton stops branching at this point. The final distribution of quarks and
gluons represents this collection of partons with a $Q=1$~GeV. The hollow circles represent the distribution of quarks, while the hollow squares represents
the distribution of gluons. Results are presented for 100,000 events.

\begin{figure}[htbp]
\resizebox{3in}{3in}{\includegraphics{g-100-Q-50-vac}}
    \caption{ (Color online) Same as Fig.~\ref{fig3} except that the originating parton is a 100 GeV gluon.
    MC results are for 100,000 events. See text for details.}
    \label{fig4}
\end{figure}

Comparison with analytic DGLAP calculations is not straightforward. One starts with a quark-to-quark and
gluon-to-quark fragmentation function at the lower scale of $Q^{2} = 1$~GeV$^{2}$,
\bea
D_{q \ra q} (z, 1~{\rm GeV}^{2} ) &=& \kd(1 - z) , \nn \\
D_{g \ra q} (z, 1~{\rm GeV}^{2} ) &=& 0.
\eea
This is then evolved up to $Q=50$~GeV to obtain the $D_{q\ra q} (z, 2500~{\rm GeV}^{2})$ and $D_{g \ra q} (z, 2500~{\rm GeV}^{2})$.
The quark-to-quark fragmentation function is plotted as the solid blue line in Fig.~\ref{fig3}. One then performs another calculation where
the starting point at $Q=1$~GeV is given as,
\bea
D_{q \ra g} (z, 1~{\rm GeV}^{2} ) &=& 0 , \nn \\
D_{g \ra g} (z, 1~{\rm GeV}^{2} ) &=& \kd (1 -z ).
\eea
These are then evolved up to $Q^{2} = 2500$~GeV$^{2}$ and the quark-to-gluon fragmentation function at this upper scale is plotted as the dashed
magenta line in Fig.~\ref{fig3}. In Fig.~\ref{fig4}, we reverse the order in the input fragmentation functions defined above to consider the
case of a gluon jet with a $Q=50$~GeV, showering in vacuum, and terminating with a distribution of quarks and gluons at $Q=1$~GeV.

As the reader would have guessed, the analytic calculations are hindered by the fact that the $\kd$-function is not
an acceptable input to the DGLAP evolution equations, as it is singular at $z=1$. This singularity has to be regulated by choosing a particular representation
of the $\kd$-function. As was noted in Ref.~\cite{Armesto:2011ht}, only one of the standard regulators where
\bea
\kd(x) &=& \lim_{\e \ra 0} \frac{1}{\e} \,\,\, \forall \,\,\,  |x| < \e, \nn \\
\kd(x) &=& \lim_{\e \ra 0} 0 \,\,\, \forall \,\,\, |x| > \e ,
\eea
has yielded convergent results as $\e \ra 0$.
In spite of such issues, the agreement between the MC simulations and the DGLAP calculations is rather good.

\begin{figure}[htbp]
\resizebox{3in}{3in}{\includegraphics{q-100-Q-50-med}}
    \caption{ (Color online) A comparison between the in-medium MC calculation and an in-medium DGLAP calculation. The medium has a length
    of 5~fm and a $\hat{q} = 1$~GeV$^{2}$/fm.
    The originating parton is a 100 GeV quark. MC results
    are for 100,000 events. }
    \label{fig5}
\end{figure}

 We next present a comparison between the MC calculations for a hard jet propagating through a dense medium and an in-medium DGLAP calculation.
 These are presented for a parton with an initial energy of 100~GeV, a $Q=50$~GeV, propagating through a medium of
 length $5$~fm with a homogeneous $\hat{q}=1$~GeV$^{2}/$fm. Fig.~\ref{fig5} represents the case of the initial parton being a quark, and Fig.~\ref{fig6}
 represents the case of the initial parton being a gluon.
  The comparison is not as good.
 This is mostly due to the approximations introduced in the in-medium DGLAP calculations, primary among which is the
 neglect of space-time dependence of the fragmentation function~\cite{Majumder:2009zu}. The result of this neglect is that the DGLAP evolutions equations
 show a higher result for $z \ra 1$ and are smaller than the MC calculations over most of the range of $z$.

\begin{figure}[htbp]
\resizebox{3in}{3in}{\includegraphics{g-100-Q-50-med}}
    \caption{ (Color online) A comparison between the in-medium MC calculation and an in-medium DGLAP calculation. The medium has a length
    of 5~fm and a $\hat{q} = 1$~GeV$^{2}$/fm. The originating parton is a 100 GeV gluon. MC results are for 100,000 events.}
    \label{fig6}
\end{figure}

As we mentioned  above, the DGLAP evolution equations show regulator dependence when the input is a $\kd$-function. To remove this defect in
the comparison, we fold both the MC calculations and the DGLAP evolutions equations with an experimentally measured hadronic
 fragmentation function. In the case of the
DGLAP evolution equations, this is straightforwardly done by replacing the $\kd$-function with a fragmentation function (in this particular case, we use a
$\pi^{0}$ fragmentation function) at the lower scale of $Q_{0}^{2} = 1$~GeV$^{2}$. In the interest of simplicity, we use the Binnewies-Kniehl-Kramer (BKK) fragmentation function~\cite{Binnewies:1994ju},
which has a simple analytic expression. This is then evolved up to the scale of $Q^{2} = 3$~GeV$^{2}$.
For the case of the Monte-Carlo calculation, there is
no straightforward means to fold a fragmentation function: one needs an hadronization model such as string breaking in PYTHIA~\cite{Andersson:1983ia,Bengtsson:1987kr} or cluster fragmentation as in HERWIG~\cite{Catani:1991hj,Marchesini:1991ch}.  Here we use a very simple \emph{ansatz}:
We allow the partons to first shower in the medium and then continue to shower in the vacuum until they reach a $Q_{0}^{2} = 1$~GeV$^{2}$.  We then convolute the BKK fragmentation function at a $Q_{0}^{2} = 1$~GeV$^{2}$ with the longitudinal distribution of final partons (as plotted in Figs~\ref{fig3}-\ref{fig6}).
Partons that reach the lower scale of $Q_{0}^{2} = 1$~GeV$^{2}$ while still deep in the medium (more than 1~fm from the exit surface) are excised from the
shower.
This hadronization set up should be accurate for the $z\ra 1$ (hard) partons which are expected to hadronize independently and become less accurate for soft partons, where one expects
several partons to participate collectively in the hadronization process.
The results of this comparison are plotted in Fig.~\ref{fig7}, where we present the ratio of the medium modified fragmentation function to the vacuum fragmentation function of $\pi^{0}$'s, from a hard initial quark. In the medium modified calculation, we have chosen a medium of length $4$~fm with a
$\hat{q}=0.2$~GeV$^{2}$/fm. This is comparable to the measured ratio of the yields of leading hadrons observed in the case of DIS on a large
nucleus to that in a proton, as seen by the HERMES experiment~\cite{Airapetian:2007vu}.
The parameters used are somewhat close to the case of the Krypton nucleus~\cite{Majumder:2009zu}. Once again, the agreement between the
two calculations is quite good. Monte-Carlo calculations are carried out for 100000 events. There are error bars associated with both the
vacuum and medium modified MC simulation, which have not been presented.
\begin{figure}[htbp]
\resizebox{3in}{3in}{\includegraphics{MC_DGLAP_comparison}}
    \caption{ (Color online) A comparison of the ratio of medium modified to vacuum fragmentation functions, as calculated by the Monte-Carlo event
    generator and using DGLAP evolutions equations. Both calculations take, as input, vacuum BKK fragmentation functions at the lower scale of $Q_{0}^{2}=1$~GeV$^{2}$. }
    \label{fig7}
\end{figure}

Having tested the Monte-Carlo simulation against analytical DGLAP calculations, we now proceed to calculate quantities that may only be
accessed via a Monte-Carlo event generator. In Fig.~\ref{fig7}, the fragmentation functions are defined in the traditional way, where the light-cone
fraction $z=p_{h}^{-}/p^{-}$ is defined with respect to the original energy of the hard parton $p^{-}$ before it enters the medium. Recently,
the CMS and ATLAS collaborations have defined the fragmentation functions in another way~\cite{ATLAS:2012ina,Chatrchyan:2012gw}.
The jet with degraded energy is reconstructed and
one then calculates the fragmentation function with the degraded total energy ${p'}^{-}$, i.e., $z' = p_{h}^{-}/{p'}^{-}$.  By degraded jet energy,
we mean that some of the energy of the jet has been lost in the medium and is not regained during reconstruction.
In all these calculations, partons whose virtuality has dropped below $Q^{2} = 1$~GeV$^{2}$ while still deep inside the medium (greater that a fermi away
from the exit surface) are excised from the shower. This is the case in both Fig.~\ref{fig7} and also in the calculations that will be described in Fig.~\ref{fig8}.

One notes that the
fragmentation functions obtained by the CMS and ATLAS collaborations are quite different (even qualitatively) from those measured by the
HERMES collaboration, in DIS on a large nucleus. For the case of HERMES, the fragmentation functions are defined with respect to the
original energy of the jet before it enters the medium and have a behavior similar to that in Fig.~\ref{fig7}, i.e., the ratio of the medium modified
fragmentation function to the vacuum fragmentation function is monotonically decreasing with increasing $z$. However, the fragmentation
functions measured by CMS and ATLAS show an initial drop and then a rise, with increasing $z$, in the ratio of the medium modified
fragmentation function to the vacuum fragmentation function. We will demonstrate that this sort of non-monotonic behavior is typical of cases
where the entire energy of the hard jet is not reconstructed, i.e., cases where some of the energy is lost in the medium.

\begin{figure}[htbp]
\resizebox{3in}{3in}{\includegraphics{survival_func}}
    \caption{ (Color online) Calculations of the ratio of the medium modified fragmentation function to the vacuum fragmentation functions for a
    quark jet and a gluon jet with an initial energy of 100 GeV, propagating through a medium of length 5~fm, with a $\hat{q} = 1$~GeV$^{2}/$fm.
    The green crosses and maroon squares represent fragmentation functions constructed using the full initial energy of the quark and gluon jet respectively.
    The remaining plots represent fragmentation functions constructed using the final degraded energy of the jet, which results from the non-detection of
    partons with energies below $2$~GeV and $4$~GeV.  See text for datails.}
    \label{fig8}
\end{figure}

In Fig.~\ref{fig8}, we plot various versions of the ratio of the in-medium fragmentation functions to vacuum fragmentation functions. In all cases,
for the medium modified fragmentation function, we have an originating quark jet or a gluon jet with an original $E=100$~GeV, and
a maximum $Q = 100$~GeV. The maroon squares and green crosses represent the case where the fragmentation functions are defined with respect to
the original jet energy, as in the case of HERMES. These represent the standard definition of the fragmentation function (with $z'=z$),
and the ratio of medium modified to vacuum shows a monotonic decrease with increase in $z$. The red diamonds and green up-triangles represent
quark and gluon jets where all partons in the shower with a forward light cone momentum below $p^{-}_{min} = 2$~GeV (i.e. $E < \sqrt{2}$~GeV)
are excluded. The jet is reconstructed from the ensemble of surviving partons and has a lower light-cone momentum $p'^{-}$.
The light cone fraction $z' = p_{h}^{-} / p'^{-}$ is defined with respect to this lower momentum. This automatically moves particles with a $p_{h}^{-} = z p^{-}$
to a higher value of the variable $z$.  Since the fragmentation functions are steeply falling with $z$, this leads to an enhancement at larger $z$.
The enhancement is larger for the case of gluons as the gluon fragmentation function is more steeply falling than the quark fragmentation function.
Increasing the threshold of partons which survive to $p^{-}_{min} = 4$~GeV, leads to a greater shift of final hadrons to higher $z$ and results in more
enhancement. Similar conclusions were also reached by a more sophisticated analysis within the YaJEM event generator in Ref.~\cite{Renk:2012ve}.

The reader will note that while qualitatively similar, these ratios of fragmentation functions do not show quantitatively the same behavior as that observed
by CMS and ATLAS. We would point out that these calculations are performed for a static brick of finite length, all medium dynamics have been ignored.
Also one does not observe quark and gluon fragmentation functions separately, but rather a mixture of the two where the amount of admixture
depends on the momentum of the detected hadrons. In future publications, these Monte-Carlo showers will be propagated through a dynamical
medium to calculate the modification of hard jets.

\section{Conclusions}

In this paper, we have presented the first Higher-Twist based Monte-Carlo jet event generator (MATTER++).
Unlike all other previous event generators, the current event generator has a space-time structure built into the
formalism. Similar to Q-PYTHIA (as well as JEWEL to some extent)
and vacuum event generators, but different from MARTINI, MATTER++ generates events by sampling
a Sudakov form factor, which is constructed by a combination of vacuum and medium modified splitting functions.
Calculations have been carried using both a truncated Guo-Wang kernel or the first positive cycle of the Aurenche-Zakharov-Zaraket
kernel. These yield similar results, if the transport coefficient is modulated with the choice of kernel.
Thus the current event generator keeps track of the virtuality of every part of the shower explicitly.

The light-cone locations ($x^{-}$ locations) of all the splits are determined by sampling the Fourier transform of the
uncertainly in the opposite light cone momentum (i.e. $\D p^{+}$). The width of the $x^{-}$ distribution is set to reproduce the
formation time of a radiation with a given $p^{-}$ and $p^{+}$. As a result, the current event generator keeps track
of the exact locations of all the splits in a given event and assuming light like propagation between splits, also can
yield the exact light-cone location of the various partons.
Transverse broadening is carried out parton by parton in the regions between the splits, with appropriate
color factors depending on the flavor of the parton. So far calculations
have been carried out assuming two undistinguished flavors of quark.

In order to simply study the behavior of the jet event generator
separated from the dynamics of the medium, we have carried out simulations on a static medium of finite length,
held at a fixed temperature. The jets are created at one end and propagate to the other end, showering in the
process. Given the lack of any transverse dynamics in the medium and the desire to not use an jet clustering
algorithms, we have not discussed the transverse structure of the hard jet. The focus has been primarily on the longitudinal
structure, which may be compared with standard DGLAP evolution routines. Using a $\kd$-function as the input parton-to-parton
fragmentation function at the scale of $Q_{0}=1$~GeV$^{2}$ as well as a regular BKK parton-to-hadron fragmentation function,
we compute and compare the longitudinal distributions of
quarks and gluons from DGLAP calculations and the MATTER++ simulations.

The comparisons for the case of the vacuum in Figs.~\ref{fig3} and \ref{fig4}, which represent the case of an originating quark jet and a gluon jet
respectively, are excellent. The comparisons with the case of the medium with a length of 5~fm and a $\hat{q}=1$~GeV$^{2}/$fm, in Figs.~\ref{fig5} and \ref{fig6},
are satisfactory, though not excellent. This is due to the somewhat different dynamics that is naturally included in a Monte-Carlo simulation versus
a DGLAP evolution calculation. For example, evolving a $\kd$-function using the DGLAP equation is somewhat difficult due to convergence issues.
Also the full three dimensional integration that is required by Eq.~\eqref{in_medium_evol_eqn}, can only be carried out approximately by averaging over the
distance dependence of the fragmentation function.

Comparisons using the BKK parton-to-hadron fragmentation function show better agreement between Monte-Carlo and DGLAP calculations.
Even this comparison is not exact as partons in the Monte-Carlo simulation which drop below the minimum
$Q_{0}^{2} =1$~GeV$^{2}$,
while more that a fermi away from the exit surface are excised from the shower. These cannot be fragmented using a perturbatively factorized fragmentation
function. Also at this low scale these interact strongly with the medium and based on AdS/CFT calculations, these should be swiftly attenuated in the medium.
We also presented a study motivated by the recent measurement of the fragmentation functions within a jet as measured by the ATLAS and CMS collaborations.
We have clearly demonstrated that if some part of the jet's energy is lost in the medium and as a result is not present in the reconstructed jet energy, then
the ratio of the medium modified to the vacuum fragmentation function shows a typical non-monotonic behavior of first decreasing with increasing $z$ and
then increasing with with increasing $z$.

The Monte-Carlo simulations presented in this paper, are rather simplistic. In future efforts, the transverse structure of the jet will be studied using jet reconstruction
algorithms. The propagation of these jets will then be studied in a dynamically evolved medium, both in smooth and event-by-event fluid dynamical simulations.
The production cross section of the jets will be calculated from the product of nuclear parton distribution functions and hard scattering matrix elements. Finally, a more phenomenologically accurate hadronization scheme will need to be used to hadronize these jets.

\acknowledgements
The author would like to thank the members of the Monte-Carlo working group of the JET collaboration for
extensive discussions. He would also like to thank Sean Gavin and Joern Putschke for helpful discussions.
This work was supported in part by the National Science Foundation under grant number PHY-1207918.
A part of the Monte-Carlo code was written while the author was employed at Ohio State University, where it was supported
by the U.S. Department of Energy under grant numbers DE-SC0004286 and (within the framework of the JET
collaboration) DE-SC0004104.


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ThingCharger - Is ThingCharger The Next Big Accessory?
ThingCharger is the most innovative and intriguing electronics accessory we have seen for some time. Its basic premise is simple, yet the efficiency it adds — both in terms of saving space and hassle — is immeasurable. This is an item that almost everyone is going to want to have in their home, particularly those who have multiple handheld devices (such as smartphones, MP3 players and tablets) and get tired of trying to negotiate outlet allotments in order to keep them charged and ready to go. ThingCharger might have a funny name but the convenience this device brings to your home is no joke.
The problem solved by ThingCharger is one that most of us can relate to: the need to power up all of our various gadgets — most importantly our mobile phones, which have become lifelines for both professional and social requirements — means that we're constantly dealing with limited outlet space, bulky charger ports and tangled cords. This leads to various problems that extend beyond the simply disorganization of it all. Placing a charging cell phone on the counter leaves it vulnerable to puddles and spills. Charging cables are prime victims for pets to chew through. ThingCharger offers a slick solution that is more than convenient — it's sharp and ultra-modern.
At first glance, the ThingCharger device looks like a standard outlet with two three-prong input spots. This is by design. It actually is an adapter that plugs into an outlet, and features an interchangeable device charger that protrudes from the top. When the ThingCharger is plugged in, it looks like the outlet did before (though a closer inspection will discover that it sticks out slightly from the wall) and you can use it as such, plugging in anything requires electricity without losing any wattage in the translation. But what makes this accessory totally unique and incredibly nice to have is that charger for mobile devices.
The mobile device charger port emerges discreetly from the top of the ThingCharger apparatus. Using it, you can take your phone, affix it to the top of the accessory, and allow it to charge while requiring no cord and taking up no extra space. Your handheld device will be held firmly in place, and with the screen facing outward, you can keep an eye on it for incoming calls and texts while it rests against the wall and charges. It's perfect for cluttered areas and any place where cables are unwanted (particularly around animals and children). It also adds a high-tech, futuristic element to your home, which guests are sure to get a kick out of.
Thanks to the ease with which you can swap out the device charger on the ThingCharger, it's easy to use it with any device, be it smartphone, tablet, etc. Whether your need is USB, mini-USB, Lightning for iPhone or what have you, it's easy to set it up for any of them and the different options can be stored conveniently inside the ThingCharger itself. There are also two standard USB inputs on the bottom for additional needs. On top of all that, ThingCharger is one of the most eco-friendly power solutions around because it cuts down on "vampire energy" that most device chargers are guilty of.
Where Can I Buy ThingCharger?
This crowdfunded product was developed and manufactured by a small company with limited resources. It is available only online. The spike in popularity for ThingCharger has caused inventory to be an issue. Orders are currently being fulfilled and shipped for those who made their purchase within the past two months. If you act now you should be able to get yours in the mail during the current or next wave but orders are backing up quickly. Click below for specific details on when you can get your ThingCharger.


What Are The Most Popular Used Cars At Auction?
Without a doubt, there are several types of cars that stand out among the crowd at a car auction. The favorite cars can change at any time, but these vehicles have proven to be popular cars over the years.
However, these car makes are popular for a reason. See what makes these vehicles stand out in the crowd.
Ferrari. According to CNBC, Ferrari dominates the car auction field. All of the top five cars are Ferrari and most of the 10 ten are as well. Anyone who has ever seen a Ferrari can see why it is a popular choice, but there are other reasons for this as well. The vehicles look great and run great. It is the ideal choice for someone looking to make a statement in the market. They are muscle cars that perform the way they claim. Some popular models are the Marque, the 275 GTB/C Speciale, and the California Spider.
Plymouth. Plymouth also makes muscle cars, which is a big reason why they are popular at car auctions. Not only are they muscle cars, but they are iconic American muscle cars. They definitely make a statement. Plymouth still makes some great vehicles, but there is nothing like a classic, which is what is typically found in car auctions all over the world. They tend to go for a lot of money at auction, but are definitely worth every cent. Some popular models are the Road Runner, the Barracuda, and the Duster.
Lamborghini. This make is special because you are able to find both vintage and modern models at any car auction. They are built for speed and are easy on the eyes. They have been designed better than many other models and some say that they were before their time, meaning they were innovative vehicles. Both today and in years prior, the Lamborghini is a prestigious vehicle. Some popular models are the Gallardo, the Aventador, and the Murcielago.
Chevrolet. This is an American classic and there are many different options when looking for Chevrolets. You can find convertibles as well as trucks that are coming to auction. Most of these are vintage vehicles, but not all of them. However, one this is for sure: people who love Chevys tend to love nothing else. Some popular models include the Impala, the Corvette Stingray, the Bel Air, and the Nova.
Ford. Ford is definitely a rival of Chevrolet. This is another American classic and they have a wide range of models that go up for auction every year. You can find both vintage and recent models of Ford at pretty much every auction you find. They are very popular. If you are a Ford lover, then you probably are all about Fords. Some popular models would be the Model A, the Mustang, and the Thunderbird.
Pontiac. Pontiac is a common name that you hear at car auctions. One great thing about Pontiac owners is that the people bringing them to auction are doing some pretty innovative things to the vehicles before they are sold. Recently, the world's first transparent car was sold at auction: it was a Pontiac. Pontiac has some great concept cars that stand out in the crowd and are definitely vehicles that are prized possessions. If you find a concept Pontiac car at an auction, you will likely want to make a bid. Popular models would include the Firebird, the Grand Prix, and the Trans Am.
There are many options to be found at car auctions both online and in person. With so many vehicles going to auction, it can be easy to get lost in the options. However, there are pros and cons to each vehicle and you will hear something different from almost every person you speak to. This is based on their personal opinions as well as knowledge of the vehicles.
When going to an auction, it is best to learn about the vehicles and make your own opinions. One person who loves Chevrolet will tell you they buy nothing else and that Ford is a joke, but you can also find someone to say the opposite. These are the top makes at auction, but you can choose your favorites based on your knowledge and personal criteria.


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Q: Tween Engine library problems on Android libgdx project This is the same problem I have read and no useful answer found,
I have libgdx, and tween engine progect,i'm working with eclipse,
I use this tutorial to install tween engine Uneversal Tween Engine
all ok, no errors, I use FileTree Dependency Method, the program run on desktop but not on android, there is no erros on the code,I
I import the project with Android studio, and the erros are
Error:(14, 33) error: package aurelienribon.tweenengine does not exist
Error:(25, 10) error: cannot find symbol class TweenManager
etc...
my project is at
C:\NovelaGrafica\codigoFonte
my tween jar files are located at
C:\NovelaGrafica\codigoFonte\libs\tween-engine-api-6.3.3
the main problens is on using the tween library,
WHAT CAN I DO,??? I have spend day looking for answers but nothing works
I'm using windows 10, eclipse Mars and android studio
HELP PLEASE!..........:(

A: I Finaly got it I just folow that tutorial Universal-Tween-Engine
with a difrence, at the end I didnt use gradlew --refresh-dependencies I use, and that is the importante point  gradlew.bat eclipse  I'm using windows10 if you are using linux I think is somethin similar probably ./gradlew eclipse
them I Close the eclipse project and import it again, this is important too
I spend 2 day for finding a solution to this ....

redpajama_set_name: RedPajamaStackExchange


Once, it was Europe's biggest water tower, now it is one of the best conversion jobs in the world. In this 130 year-old building, you will stay inside a design job worth $75 million. The 11 meter high lobby is as impressive as the collection of art hanging on the walls, including pieces by Warhole. You room is designed to fit into the architecture and you will find a marvelously mosaic bathroom of marble. Floor-to-ceiling windows are a common sight. Or if you are in the top suites, you will have the use of two floors, soundsystem and whirlpool. The hotel hosts the annual trade fair for the confectionary industry featuring a keynote speech by Augustus Gloop. Only joking. There are loads of unique and unusual museums and sights of historical interest to arouse your curiosity when exploring the local area. You can enjoy amazing views in the 2 Michelin starred restaurant on the top floor serving contemporary German cuisine and in summer you can sit outside on the roof terrace.


4 Adjustable Brightness Settings; Four Extra-Bright, Energy-Efficient LEDs.Flexible Goosenecks Put Light Exactly Where Needed on your Music Stand.
Individual Light Switch on Each Head – with Two Light Levels Per Head, for Total Control.Engineered Lens Distributes Light Precisely on your Music Stand. Portable Lights for Musicians, Artists, Crafters and Readers, Ideal Accessories for BBQ, Mixing, Work, Craft, Travel and Desk.Free AC Adaptor/USB Cord Incl. AAA Battery Powered (Not Included).


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— Décembre 9, 2019
Kentucky law requiring abortion seekers to listen to fetal heartbeat will stand
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Province launches Ottawa's first Health Team
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Cellphone Distraction Linked To Increase In Head Injuries
Most people understand the dangers of texting and driving, Amato said, but the risk of serious head ...
Seychelles launches HIV self-test programme on World AIDS Day
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Bernie Sanders pulls ahead of 2020 Democratic presidential rivals in California
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redpajama_set_name: RedPajamaCommonCrawl


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Rep. Bob Rankin — Under the Dome: Thanks to my constituents
News | May 16, 2014
Rep. Bob Rankin/For the Saturday Morning Press
Colorado House District 57 Rep. Bob Rankin, R-Carbondale
The House and Senate conducted a memorial for former Gov. John Vanderhoof that I was honored to present. The future governor came to Glenwood Springs as a World War II veteran recovering from his wounds and stayed to become a leading businessman, state representative for 20 years (before term limits) and governor. Two former governors and the current governor spoke in the House chamber in memory of Vanderhoof with nine family members in attendance. Colorado's history and traditions come alive through these memorials and are valued by every member of the Legislature.
My House caucus backed me aggressively in a floor fight about a bill that will take $6.5 million from the federal mineral lease fund to pay for a statewide firefighter equipment grant program. Federal and state statues are clear about the intended use of these funds generated by mineral development on public lands. I proposed an amendment to instead use general fund monies but once again, we are outnumbered by urban interests and the majority party. Our western counties contribute substantially to state revenues through these federal mineral lease funds and severance taxes without, in my estimation, receiving appropriate benefits.
I sponsored the species protection bill, a yearly allocation of funds to the Department of Natural Resources, which will allow the department to continue its effort to protect wildlife and also prevent inappropriate listing of species as endangered. The department has implemented species protections aggressively for years with some success and is working hard on greater sage grouse protections while negotiating with the U.S. Fish and Wildlife Service to avoid major economic impacts from a listing.
I'm very concerned about the future of Garfield County's economy and jobs. The county is facing twin crises of declining gas production and the highest health care rates in the nation. With mandatory coverage under the Affordable Care Act, residents of Garfield County are losing coverage and can't afford to replace their canceled policies. Despite the tireless efforts of Garfield County Commissioner Tom Jankovsky, the state is not likely to make more than a small improvement in insurance rates for next year. Meanwhile the Bureau of Land Management is signaling not only fewer new drilling permits on federal lands but even a reversal of leases that have been in place for years. Combined with low prices for gas and competition from states with less costly regulation, we can expect the energy sector of the economy to decline. And new businesses that might replace energy will have a choice of locating in Grand Junction or Boulder, where their health care costs are 50 percent less.
I was recently appointed to the Joint Budget Committee. The JBC is made up of six representatives and senators who are responsible for the state's final budget after input from the governor's office and the Legislature. I plan to advocate for rural Colorado and the Western Slope but also work hard to help manage the $20 billion spending machine that is Colorado government. This is an important assignment, but I'll have to give up my roles on the Agriculture and Natural Resources Committee, the Local Government committee and the Technology Committee.
Thanks to all of the residents of District 57 for your confidence and support. I take seriously my obligation to support all of us, regardless of party affiliation. We won't always agree, but I'll continue to explain my position and represent your interests.
State Rep. Bob Rankin, R-Carbondale, represents House District 57, encompassing Garfield, Moffat and Rio Blanco counties.


Gæster, der rejser med et servicedyr, skal kontakte ejendommen før ankomsten. Kontakt overnatningsstedet via oplysningerne angivet i reservationsbekræftelsen.
Bed was hard, but so were all the beds in Japan. Pillows were hard and one side were rows of cut plastic tubing. Quite strange. Breakfast was , ok, but the powdered eggs need to be rethought, or have some salt and pepper.
Great hotel, walkable distance from Kyoto Station!
Fantastic hotel! Relatively close to the Kyoto Station, so walking is definitely a 15 min option. The hotel staff was extremely kind and very accommodating. The location of the hotel was easy enough to walk to most places that we wanted to get to, like Kyoto tower, Gion, etc. The room size is great for two people. Considering I am from the US and the standard size of those rooms is much larger than this, you'll just have to adjust your perspective and expectations and you'll be pleasantly surprised. Overall, excellent hotel and staff, would recommend to others and would book again if the opportunity was available!
Brand new modern hotel at a great price!
Don't hesitate to book this awesome hotel in Kyoto that is just a 10 minute walk from the Kyoto station. The hotel staff are very kind and helpful and the rooms equipt with everything you need, air con, safe, hairdryer, bathroom products, slippers , tea/coffee making facilities etc. The bed was really comfortable and the shower nice and hot. Although we didn't eat breakfast in the hotel it looked delicious. The lobby also had free tea and coffee which we did enjoy. Don't think just book this place, you'll be very happy!
What a lovely welcome received from a very smiley receptionist. Extremely friendly and helpful. It is about a 10-15min walk to the main station. The room is on the smaller side but very typical for Japan. Very clean. Would recommend!


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A message from Judy Marsales about COVID-19
We are focussed on continuing to serve our communities in this time of need.
We are committed to doing our best to continue helping you navigate through this challenge and this includes providing you with real estate services while protecting the health and well-being of our staff, sales representatives, independent contractors and customers. However, we recognize that many of you may have pressing real estate needs which must be dealt with irrespective of COVID-19. Rest assured that we are here for you, ready and able to accommodate your needs, with health and safety being our top priority. We have made some adjustments to how we conduct business and associated real-estate transactions.
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Hamilton Music Festival - April 17 to 28 2017
Tuesday, April 18, 2017 Judy Marsales Community Events
Special Fundraiser… the committee's students are performing a fundraising concert at St. Pete's HARRRP, 705 Main East.
Amazing young musicians to support – Free Will Offering.
This year we have added Strings and have increased the festival run from 5 days last year to 10 days this year. April 17 to 27.
Our Web site is www.hamiltonmusicfestival.ca
Venues are all in the Locke Street area. There is a $3.00 fee to see these wonderful performances. We hope that the community will come out and support these performances.
Hamilton had been without a festival for about 15 years. Co founder, Diane Manojlovich (Mano Music Studio - piano studio) and myself Tom Oliver (Voice Concepts Music Studio) brought 10 colleagues together to re introduce the festival to the community.
Last year about 30 private music studios were represented and this year over 60 private music studio are represented with approximately 600 entrants.
We are thrilled to have the blessings of the Mayor's office and many sponsors, including the Hamilton Duet Club, and Judy Marsales Real Estate Ltd.
This Saturday April 15 at 7:30 pm, the committee's students are performing a fundraising concert at St. Pete's HARRRP, 705 Main East. Free Will Offering.
We are close to raising 10 K for scholarships.
NOTE: Hamilton has also been selected to host the PROVINCIAL MUSIC FESTIVAL this JUNE. We are absolutely thrilled that our inaugural year had such an impact. The Provincial competition will be housed in ten venues throughout Hamilton downtown core. It will feature students from regional festivals selected by adjudicators to compete. It is such an honour and at the same time a huge project to organize. Diane Manojlovich has offered to organize the event. However, our Hamilton Music Festival Committee will all volunteer to help her with this enormous task.
Festival at a Glance
First Unitarian Church on Dundurn
Monday April 17, 1 pm to 8 pm - Senior Piano
Tuesday April 18, 9 am to 5 pm - Senior Piano
Wednesday April 19, 9 am to 9 pm - Senior Piano
Thursday April 20, 9 am to 5 pm - Junior Piano
Friday April 21, 9 am to 4:30 pm - Junior Piano
Saturday April 22, 1 pm to 4:30 pm Orchestras
St. John's the Evangelist "Rock on Locke" on Locke Street.
Monday April 17, 9 am to 5 pm - Junior Voice
Tuesday April 18, 9 am to 4:30 pm - Junior Voice
Wednesday April 19, 2 pm to 9 pm - Senior Music Theatre
Thursday April 20, 12:pm to 5:30 pm - Senior Music Theatre
Friday April 21, 9 am - 9 pm - Strings
Saturday April 22, 9 am - 11 am - Strings
Monday April 24, 9 am to 5 pm - Senior Classical Voice
Tuesday April 25, 1 pm to 9 pm - Senior Classical Voice
Wednesday April 26, 9 am to 9 pm - Junior Music Theatre
Thursday April 27, 9 am to 4 pm - Junior Music Theatre
Erskine Presbyterian Church - Pearl Street.
Wednesday April 19, 9:30 to 12:15 pm Senior Music Theatre
Monday April 24, 7 pm to 9 pm Senior Classical Voice
GRAND CONCERT OF RECOMMENDED PERFORMANCES
Saturday May 6, 7 pm at the Grand Hall, Conservatory of the Performing Arts, James St.
Community Events 1
Community events in and around Hamilton
General Real Estate Advice 30
Tips and Advice for the those interested in or involved in the purchase or sale of real estate.
Investment Properties 1
Information, tips and advice on Investment Properties
Local Hamilton Market Statistics 30
Information and updates about the Greater Hamilton Area Real Estate market conditions
Real Estate Trends 15
Trends in Canadian real estate market
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A dead and looking very dangerous tree on the road side. Who would be the best persons to deal with this please.. ? Old Cherry maybe, about 400mm at the bottom and probably 15/20M high.
07/02/2019 I am the occupier of 61 West Chiltern and have been away for 3 weeks. The dead tree mentioned above (reported by someone else in January) has leaned further towards the south since I left and I am concerned that if it falls it will cause injury to passers-by or damage parked cars. I think the weather forecast is for high winds over the next few days. Please feel free to email me for further clarification if you wish.
The update reads "State changed to: No further action" and my interpretation is that nothing more will be done despite there being a large red cross on the tree. May I assume therefore that if the tree falls unexpectedly the council will accept liability for any damage to passers-by or vehicles?


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By Homestead News On Jan 19, 2023
MUSCODA – I wonder if there is any subject that generates more conversation than the weather of the moment. If you meet a co-Muscodite at the grocery store, post office, church, or wherever, the conversation usually starts with, "Nice Day!" or "I hate these damp cold days!" Whether the weather is good or bad, it seems to always generate a hot or cold comment.
A cousin and I share a telephone line quite often with the exchange centered on weather. He lives near the western end of Nebraska, an area that has recently seen major highways closed for numerous days because of snow, sometimes coming as dayslong blizzards.
Weather may be a factor when deciding where we live. Many years ago I had a great-uncle and aunt who spent their summers in Nebraska and winters in Florida. They were retired Nebraska farmers and relatives would ask them, "Why do you go to Florida where they have hurricanes?" Uncle Clint would reply, "I would rather experience a Florida hurricane than go through a Nebraska blizzard."
Some people may disagree with that logic. When Vi and I sat in our warm living room and recently witnessed, through television, the destruction of homes and businesses in the South by wind and water, she opined, "At least the snow doesn't come in the house and get you!"
I have never been in a hurricane, but I do remember Nebraska blizzards and they can be killers as people get lost, sometimes close to home, but can't find it. Vi recalls a blizzard when her mom sat in a window, with prayer book inhand, waiting for husband to show up through the wind-driven snow, carrying a calf he went to rescue. Everyone survived and the calf became a cow named "Frosty."
One of the historic weather events in this area was the Armistice Day Blizzard of 1940. I have written about it in the past and continue to be interested in stories it generated. The late Mel Ellis, Milwaukee Journal outdoor writer, reported 39 Mississippi River duck hunters died in the storm, as did more than 75 Lake Michigan sailors. A couple of Muscoda duck hunters told me about leaving the local river bottoms because of the storm.
Recently I was gifted with a new book titled "In the Grip of the Whirlwind – The Armistice Day Storm of 1940", written by Tom Powers. It's filled with stories of bravery and graphic sadness. It notes when the storm hit Chicago the damage resembled that which was taking place on the other side of the world when the Germans bombed English cities, early in World War II.
On the lighter side the book tells about an unusual football game that took place that day in Minnesota. It was an afternoon contest with the Winona High School team traveling to Rochester. When the game started there were 600 fans present, but as the storm hit, only about 75 spectators were still in the stands at the half. They saw what may be the most unusual high school game ever. It was topped off in the third quarter when the Winona punter was called into action. Witnesses said when the ball gained altitude going into the wind it just hung in the air, like a kite, until it came back to earth behind the punter. Rochester won the game 13-6 and the Winona team and fans spent the night in Rochester.
That story prompted my memory. The Nebraska winter of 1948-49 was bad, perhaps the worst. I was in high school playing basketball and can recall home teams would contact their fans and line up places where visiting fans and players could stay if a snow-moving storm came up as the game was being played. That never happened, but it was a risk.
Perhaps reading the Armistice Day book could make you a bit more cautious about challenging predicted stormy weather, even with the much improved forecasting we now experience.
Florida City family asking for community's help after house fire – WSVN 7News | Miami News, Weather, Sports
Seffner's Soulful Flavors moves to new Tampa location in University area | Openings & Closings | Tampa


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Home / India News / In clear rejection of NRC, Nitish Kumar points to PM Modi's clarification
In clear rejection of NRC, Nitish Kumar points to PM Modi's clarification
Nitish Kumar and his party had supported the Citizenship Amendment Act in Parliament's Winter session in December last year.
Hindustan Times, Patna
Bihar Chief Minister Nitish Kumar.(PTI)
Chief Minister Nitish Kumar on Monday equivocally dissed the National Register of Citizens project, telling the Bihar assembly that there was no question of rolling out the citizens' register. The citizens' register, he told a boisterous opposition that wanted a special session to be convened to discuss NRC and NPR, had always been only envisaged in the context of Assam and not the entire country.
Kumar, however, did not give any commitment on the population register project which, his deputy in the government Sushil Modi has announced, will begin on May 15 and continue till May 28.
Opposition-ruled states such as West Bengal and Kerala, have declared that they will not allow the population register either since it was meant to create the mother database that will be used to build the citizens' register. Opposition parties such as Tejashwi Yadav's Rashtriya Janata Dal and the Congress wanted Nitish Kumar to block the population register also, particularly since the Centre was likely to increase the number of questions including during the nationwide census.
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One question that has particularly drawn the opposition ire relates to the date and place of birth of parents. This question is seen to have been incorporated to use the population register for the NRC.
Nitish Kumar did not take a firm stand on the population register.
"If there is any new addition to NPR, I will find out," he said.
The chief minister said he was completely involved with the Jal-Jeevan-Hariyali yatra across the state that will culminate with a human chain across the state on January 19.
"After January 19, I will look into all the points which the leaders have raised again," he said.
This is the first time that Chief Minister Nitish Kumar has clearly spoken against the citizens' register.
The only other time he had spoken about the citizens' register was last month when he responded to a question about NRC with a counter-question. "Why will it be implemented in Bihar," Nitish Kumar had said on December 20, a remark that was seen to indicate that he was not on board with the Centre's plan to roll out a nationwide citizens' list.
https://www.hindustantimes.com/india-news/no-question-of-nrc-says-nitish-kumar-yet-to-firm-up-stand-on-new-npr/story-yCj8myVRu23U6T8dBCEwaP.html


If Lord Krishna of infallible will, the Supreme Lord of all, and in whose control the entire phenomenal display of the total material creation is created, maintained and preserved by His inconceivable potency; if He were not to conduct Himself seriously and omit to perform prescribed Vedic activities for the benefit of all the worlds then others seeing Lord Krishnas indifference would also conduct themselves indifferently following His example. When Lord Krishna took birth, seemingly as a human being, as the son of the great righteous King Vasudeva, he conducted Himself in all ways and manners as appropriate for his position in society as a prince of the royal ksatriya or warrior class. If Lord Krishna acted otherwise all mankind would begin to imitate Him thinking that such actions were virtuous, the worthy actions, of a worthy son from a worthy father, the righteous King Vasudeva. In this way Lord Krishna is explaining that if He failed to perform Vedic activities mankind following His example would be led in a negative way into a hellish perdition unable to purify themselves enough so they could achieve atma-tattva or soul realisation. This would be considered as a very serious offence and Lord Krishna would be at fault. By not setting the example of what is righteous and by not following the traditions and customs established by performing the activities prescribed in the Vedic scriptures then all humanity would deviate from righteousness and become totally lost. If Lord Krishna failed to respect the injunctions and prohibitions of the Vedic scriptures then all the world would take that to be the standard of righteousness and the final verdict. There would soon ensue the mixing of classes and a mixture of moral and immoral standards in the class of pure and righteous people, leading to the complete degradation of society. Lord Krishna is stating that if He failed to follow and perform the Vedic injunctions then it would be the cause of the destruction of society. This is the purport. Also if Arjuna who was world famous for never having been defeated in battle and who was the brother of King Yudhisthira famed for his righteousness; if Arjuna refused to fight and protect dharma or righteousness then many other worthy and noble ksatriyas who were protectors of dharma might folow his example and also renounce their prescribed duties and refuse to protect righteousness then this would bring destruction to the world balance and ruination to the welfare of the people. Thus it can be understood that for specially qualified people prescribed Vedic activities must be performed for the benefit of the entire human race and the welfare of the world.