text:
De Sint-Pietersbandenkerk is de parochiekerk van de tot de Oost-Vlaamse gemeente Erpe-Mere behorende plaats Erondegem, gelegen aan Erondegemdorp.

Geschiedenis
In 1142 werd voor het eerst melding gemaakt van een kerk in Erondegem. Het patronaatsrecht berustte sinds 1106 bij de Sint-Adriaansabdij te Geraardsbergen.

De huidige kerk bezit een 14e-eeuws gotisch koor en een 16e-eeuwse vieringtoren. Het schip werd in 1848-1849 gebouwd.

Gebouw
De georiënteerde kerk heeft een bakstenen driebeukig schip. Het vlakafgesloten koor en de vieringtoren werden in zandsteen uitgevoerd. De toren heeft een hoge ingesnoerde naaldspits.

Interieur
Het koor wordt overkluisd door een tongewelf van 1739. Het hoofdaltaar is 18e-eeuws, met een 17e-eeuws tabernakel. Het zuidelijk zijaltaar is van 1750, getuige een chronogram, en is gewijd aan Sint-Hubertus. Een koorbank en een biechtstoel zijn 18e-eeuws en de preekstoel is 19e-eeuws. Het doopvont is uit de 17e eeuw. Er is een relikwie van Sint-Hubertus en een 17e-eeuws schilderij verbeeldt de Bekering van Hubertus.

Pietersbandenkerk
Onroerend erfgoed in Erpe-Mere

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Celebrating 40 Years of Multi Image Group
The History of MIG
Established in 1979, Multi Image Group (MIG) is a corporate event production company located in Boca Raton, Florida. This August, MIG is proud to celebrate 40 years of business with clients across the world. Over these four decades, MIG has continually evolved and always adapted to technology advancements. Beginning with projectors and 35mm slides to create multi-image slideshows, in 1979, MIG was the first off-site producer in the country to introduce computer-generated slides visuals to clients for events. The company began as a startup in the home of Jim and Arlene Sclafani.
The Legacy of MIG
Fast-forward to today, in 2019, MIG is home to 130+ technical professionals and creative visionaries all under one roof. MIG is now a third-generation, family run and woman-owned business. Every year, we continue to expand our services and serve our clients' event production needs. MIG has a history of producing shows of all shapes and sizes. From intimate corporate meetings and stadium-size live events, or busy exhibit halls and virtual reality spaces, we are the experience makers. When you partner with MIG, you'll see what it's like working with an event production company that has 40 years experience in creativity and technology.
Download Infographic Timeline
More about MIG
MIG travels the world to source the latest in event and trade show technology. By combining this technology with our creativity and experience, we are able to develop custom solutions to make audience engagements more educational, inspirational, interactive, and ultimately transformational. We consistently invest in our staff's ability to remain ahead of the curve by sending them to industry events, conferences, think tanks, and seminars. While our primary business focus is North America, MIG has worked in more than 35 countries, produced and staged over 175+ international meetings in 80+ premier venues around the globe. By providing an inclusive and open work environment, we encourage our people to share their unique abilities, embrace different ideas, approaches, and experiences in every project they touch.
MIG Puerto Rico Hurricane Relief Efforts MIG Tips for Establishing Traditions in the Workplace MIG Becomes Sole U.S. Partner of Aquatique Show International

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text:
\section{Introduction \label{sec1}}

The on going search for new physics (NP)
is mostly inspired by the
shortcomings of the SM in addressing some of the fundamental
questions in modern particle physics, such as the
hierarchy problem,
the flavor patterns in the fermionic sector and dark matter.
Some of these unresolved issues may be closely related
and may have TeV-scale origins, thus inspiring the search
for TeV-scale NP, both theoretically and experimentally.
Indeed, two seemingly unrelated interesting measurements of
both the ATLAS \cite{ATLAS1,ATLAS2} and the CMS \cite{CMS1,CMS2}
collaborations at CERN, have been recently reported:
\begin{enumerate}
\item A possible $(2-4) \sigma$ (local) excess in the diphoton invariant mass distribution
around 750 GeV,
corresponding to a signal cross-section roughly in the range
$\sigma(pp \to \gamma \gamma) \sim 3-13$ fb $(1\sigma)$, see e.g.,
\cite{1512.05777,1601.04751,1605.09401}.
The interpretation of this excess signal has a slight preference
to a spin 0 resonance, produced via gluon-fusion and having a total
width ranging from sub-GeV to 45 GeV, with a more significant signal
obtained in the ATLAS analysis for a scalar with a total width
$\Gamma \sim 45~{\rm GeV}$ \cite{ATLAS1}.
\item A possible $(1-2.5) \sigma$ excess in the measurement of the LFV decay
$h \to \tau \mu$ of the 125 GeV light Higgs. In particular,
the CMS collaboration finds $BR(h \to \tau \mu) = 0.84\%^{+0.39\%}_{-0.37\%}$ \cite{CMS2},
while the ATLAS collaboration finds $BR(h \to \tau \mu) = (0.53 \pm 0.51)\%$ \cite{ATLAS2}.
\end{enumerate}

Whether or not these two measurements are confirmed, it emphasizes the importance of the current
efforts in the search for NP, since it provides an interesting manifestation/example
of the exciting possibility that the building blocks of new TeV-scale physics may
have rather non-conventional properties, potentially with important repercussions for both flavor and the hierarchy
problems. For example, the new heavy scalar particle, $S$,
responsible for the 750 GeV $\gamma \gamma$ excess,
should have a rather narrow width and suppressed decay rates
into ``conventional" channels such as $S \to WW,~ZZ,~t  \bar t$,
for which no excess signals
has been observed within the currently available sensitivity of the corresponding LHC searches.
In addition, such a heavy scalar $S$ is most likely related
to the light 125 GeV scalar state and, therefore,
might also be involved in flavor changing (FC) transitions in the fermionic sector.
Such properties of the would be new 750 GeV resonating particle
are, therefore, very challenging to accommodate in models beyond the SM,
in particular, in supersymmetric models or in models that involve
extra space-time dimensions, which seem to have a more fundamental origin and, therefore,
likely linked to physics at higher energy scales.
Nonetheless, we will show in this paper that a certain class of low-energy effective 2HDM
frameworks with a 4th generation of heavy chiral fermions may be interesting
candidates for such ``exotic" TeV-scale NP.

In particular, since no evidence for such fundamentally structured theories has yet been seen,
a frequently adopted phenomenological approach in studies of NP,
is to construct TeV-scale models
which require a UV completion and may, thus, be
viewed as low energy effective frameworks for the underlying dynamics.
Such models are useful
as a guide for the exploration and model building of more fundamental theories and they
often include new heavy fermionic and scalar states with
sub-TeV masses. One of the simplest variants of an effective low-energy NP candidate, which dates back to the 1980's
\cite{SM4proc}, is the SM with an additional 4th generation of fermions; the so called SM4
(for useful reviews see e.g., \cite{sher0}).
Indeed, since three generations of chiral fermions have been observed in nature,
it is natural to ask why not four generations of chiral fermions?
It is quite interesting that this simple extension of the SM may address
some of the theoretical challenges in particle physics, such as:
electroweak symmetry breaking (EWSB) and the hierarchy problem \cite{DEWSB},
the CP-violation and the strength of the first-order phase transition needed
to explain the origin of matter - anti matter asymmetry in the universe \cite{baryo-ref,fok},
and flavor physics \cite{flavor}.
As is well known, the SM4 (i.e., with four generations of fermions and one Higgs doublet)
is now excluded, since it cannot accommodate
the measured SM-like properties of the 125
GeV scalar, see e.g., \cite{SM4-Higgs-bound,Lenz},
primarily due to an ${\cal O}(10)$ enhancement in the gluon-fusion light Higgs production mechanism
from diagrams with $t^\prime$ and $b^\prime$ in the loops \cite{Kribs_EWPT}; see, however, W.-S. Hou in \cite{1606.03732}.

This fact, along with the rather stringent direct limits on the masses
of such heavy quarks (to be discussed later), has led
to a common belief that generic extensions to the SM with
heavy chiral 4th generation fermions
$t^\prime,b^\prime,\nu^\prime,\tau^\prime$ are excluded.
However, as was suggested by us a few years ago
\cite{ourpaper1} and will be demonstrated again here,
this is not the case when the heavy
4th generation chiral sector is embedded in frameworks with an extended Higgs sector (see also \cite{1312.4249}).
Indeed, an extended Higgs sector in the context of 4th generation heavy fermions may come in handy
for further addressing flavor problems \cite{ourpaper1} and the strength of the EW phase transition required for
baryogenesis \cite{fok,1401.1827}.
In particular, we will consider in this paper a version of a 2HDM introduced by us in \cite{ourpaper1}
 - the so called 4G2HDM of type I, where
a chiral 4th generation doublet of heavy fermions (quark and lepton) is
added and is coupled {\it only} to one of the scalar doublets
(the ``heavy" doublet), while the SM 1st-3rd generations fermions
are coupled only to the other doublet (the ``light" doublet).
We will show in this paper that this 4G2HDM
is a well motivated and valid low-energy model,
which is compatible
with the 125 GeV signals (see also \cite{our125}), with PEWD and with the
existing direct bounds on the heavy fermions, and at the same time
can also accommodate the recent indications for a new 750 GeV scalar resonance
in the $\gamma \gamma$ channel.

As was shown in \cite{ourpaper1}, the price to pay when adding
another heavy SM-like chiral fermion doublet is that
such constructions posses a nearby threshold/cutoff at the several TeV scale,
which is manifest (as Landau poles) in the evolution of the Yukawa and Higgs
potential couplings \cite{ourpaper1,ourhybrid}.
Indeed, the large Yukawa couplings of the heavy chiral fermions can be thought of as a reflection
of an underlying TeV-scale strong dynamics, so that
the 4G2HDM framework should be viewed as a low energy (i.e., sub-TeV)
effective model of an underlying strongly interacting sector.
In particular, if the new heavy chiral fermions are viewed as the agents
of EWSB (and are, therefore, linked to
strong dynamics at the nearby TeV-scale,
see e.g., \cite{DEWSB-heavyF,luty}),
then more Higgs particles, which may be
composites of these 4th generation fermions, are expected at the sub-TeV
regime.$^{[1]}$\footnotetext[1]{Early
attempts in this direction investigated
the possibility of using the top-quark as the
agent of dynamical EWSB via top-condensation \cite{top-con}.
These models, however, fail to reproduce the observed value
of the top-quark mass. Moreover, as opposed to the case of condensates
of the heavy 4th generation fermions, where the typical cutoff for the new strong interactions
is of ${\cal O}(1)$ TeV,
the top-condensate models require
a corresponding cutoff many orders of magnitudes larger than $m_t$,
i.e., of ${\cal O}(10^{17})$ GeV, thus resulting in a severely fine-tuned
picture of dynamical EWSB.}
In such scenarios
the resulting low-energy effective
theory may contain more than a single composite Higgs field
\cite{ourpaper1,luty,DEWSB-multiH}
and may thus resemble a two (or more) Higgs doublet framework
(for other related studies of the phenomenology of multi-Higgs 4th generation models
see e.g., \cite{4G2HDM-others}).

The purpose of this work is to revisit
the 4G2HDM of \cite{ourpaper1}, studying its compatibility with the updated
measurements of the 125 GeV light Higgs signals and with
PEWD. We will also confront our model with
the 750 GeV $\gamma \gamma$ excess and study its compatibility with
a sub-percent branching ratio of the light Higgs in the FC decay channel $h \to \tau \mu$.
Indeed, many interesting and exotic constructions beyond the SM
have been suggested  as possible explanations
of the 750 GeV $\gamma \gamma$ excess (too many to be cited here); in most cases involving
new degrees of freedom beyond just the 750 GeV resonating particle.
In particular, the relevance of 2HDM frameworks to the 750 GeV $\gamma \gamma$
excess has been intensively studied in the past
several months, where it was shown
that the simplest 2HDM extension to the SM, in which
no additional heavy degrees of freedom are added
 (i.e., beyond the extended scalar sector), cannot
accommodate the necessary enhancement in $\sigma(pp \to H(750) \to \gamma \gamma)$,
see e.g., \cite{gilad}.
Consequently, extended 2HDM models with TEV scale vector-like (VL) fermions have been suggested
for addressing the 750 GeV resonance signal \cite{2HDMVLQ}.
The upshot of these studies is that, the needed
enhancement in the 1-loop production and decay channels $gg \to H(750)$
and $H(750) \to \gamma \gamma$, requires several
copies of VL fermions and/or VL fermions with charges appreciably larger
than those of the SM fermions, unless
their Yukawa couplings are much larger than one.
The 4G2HDM considered in this work
is, therefore, conceptually simpler, relying on new heavy
fermionic degrees of freedom with properties similar to the SM fermions
in a model that already exists in the literature.

The paper is organized as follows: in section 2 we describe the type I 4G2HDM and we layout
the physical parameters that are used in the numerical analysis. In section 3 we show our
results and in section 4 we discuss their phenomenological consequences. In section 5 we discuss our results and summarize.

\section{The 4G2HDM: a 2HDM with 4th generation fermions \label{sec2}}
Motivated by the idea that TeV-scale scalar degrees of freedom may emerge as composites associated with
heavy fermions, we assume that the low-energy (sub-TeV) effective framework is parameterized by a 2HDM
with a chiral SM-like 4th generation of heavy fermions. Specifically, the model is constructed following
\cite{ourpaper1}, such that
one of the Higgs fields ($\phi_h$ - the ``heavier" field)
couples only to the new heavy 4th generation fermionic fields,
while the second Higgs field ($\phi_\ell$ - the ``lighter" field)
is responsible for the mass generation of all other (lighter) fermions (i.e., the 1st-3rd generation SM fermions).
In this model, named in \cite{ourpaper1} the 4G2HDM of type I (here we will refer to it simply as the 4G2HDM),
the Yukawa interaction Lagrangian can be realized in terms of a $Z_2$-symmetry
under which the fields transform as follows:
\begin{eqnarray}
  \Phi_{\ell}\to-\Phi_{\ell},~ \Phi_{h}\to+\Phi_{h},~ F_{L}\to+F_{L}~,
  f_{R}\to-f_{R}\;(f={\rm SM~fermions}),~f^\prime_{R}\to +f^\prime_{R}\;(f^\prime={\rm 4th~gen.~fermions})~,
\label{eq:z2}
\end{eqnarray}
where $F_L$ and $f_{R},f_R^\prime$ are the SU(2) fermion (quark or lepton) doublets and singlets, respectively,
and $\Phi_{\ell,h}$ are the two Higgs doublets
$\Phi_i =\left( \phi^{+}_i,\frac{v_i+\phi^{0}_i}{\sqrt{2}} \right)$, $i=\ell,h$.

The Yukawa potential that respects the above $Z_2$-symmetry  is:
\begin{eqnarray}
\mathcal{L}_{Y}= -\bar{F}_{L}
\left( \Phi_{\ell} Y_d^f \cdot \left( I-{\cal I}
\right) +
\Phi_{h}Y_d^f \cdot {\cal I} \right) f_{d,R}
-\bar{F}_{L}
\left( \tilde\Phi_{\ell} Y_u^f \cdot \left( I - {\cal I} \right) +
\Phi_{h} Y_u^f \cdot {\cal I} \right)
f_{u,R} + h.c.\mbox{ ,}
\label{eq:LY4G}
\end{eqnarray}
where $f_{u,R}$ and $f_{d,R}$ are the up and down-type SU(2) fermion singlets (quark or lepton of all four generations),
$I$ is the identity matrix and ${\cal I}$ is the diagonal $4\times4$ matrix
${\cal I} \equiv {\rm diag}\left(0,0,0,1\right)$.

The scalar sector contains five massive states: a charged scalar $H^+$, a CP-odd
state $A$ and two CP-even scalars $h,H$, so that $h$ is the lighter one,
corresponding to the observed 125 GeV Higgs boson. These physical states are
related to the components of the two SU(2) scalar doublets via:
\begin{eqnarray}
H= s_\alpha {\rm Re} \left( \phi_h^0 \right) + c_\alpha {\rm Re}\left( \phi_\ell^0 \right)
~&,&~
A= s_\beta {\rm Im} \left( \phi_\ell^0 \right) - c_\beta {\rm Im}\left( \phi_h^0 \right)
~, \nonumber \\
h= c_\alpha {\rm Re}\left(\phi_h^0\right) - s_\alpha {\rm Re}\left(\phi_\ell^0\right)
~&,&~
H^+= s_\beta \phi_\ell^+  - c_\beta \phi_h^+
~, \label{Higgsangles}
\end{eqnarray}
where $s_\alpha(c_\alpha)=\sin\alpha(\cos\alpha)$, $\alpha$ being the Higgs mixing angle in the CP-even sector and $s_\beta(c_\beta)=\sin\beta(\cos\beta)$, where $\tan\beta \equiv v_h/v_\ell$ is the
ratio between the VEV's of the heavy and light Higgs fields.

The Yukawa Higgs-quark-quark interactions in the 4G2HDM are (similar
terms can be written for the leptons) \cite{ourpaper1}:
\begin{eqnarray}
{\cal L}(h q_i q_j) &=& \frac{g}{m_W \sin 2\beta} \bar q_i \left\{ m_{q_i} s_\alpha s_\beta \delta_{ij}
- \cos(\beta -\alpha) \cdot
\left[ m_{q_i} \Sigma_{ij}^q R + m_{q_j} \Sigma_{ji}^{q \star} L \right] \right\} q_j h \label{Sff1}~, \\
{\cal L}(H q_i q_j) &=& \frac{g}{m_W \sin 2\beta} \bar q_i \left\{ -m_{q_i} c_\alpha s_\beta \delta_{ij}
+ \sin(\beta -\alpha)\cdot
\left[ m_{q_i} \Sigma_{ij}^q R + m_{q_j} \Sigma_{ji}^{q \star} L \right] \right\} q_j H ~, \\
{\cal L}(A q_i q_j) &=& - i I_q \frac{g}{m_W \sin 2\beta} \bar q_i \left\{ m_{q_i} s_\beta^2 \gamma_5 \delta_{ij}
- \left[ m_{q_i} \Sigma_{ij}^q R - m_{q_j} \Sigma_{ji}^{q \star} L \right] \right\} q_j A ~,
\end{eqnarray}
\begin{eqnarray}
{\cal L}(H^+ u_i d_j) = \sqrt{2} \frac{g}{ m_W \sin 2\beta} \bar u_i \left\{
\left[ m_{d_j} s_\beta^2 \cdot V_{u_id_j} - m_{d_k}
V_{ik} \Sigma^{d}_{kj} \right] R + \left[ -m_{u_i} s_\beta^2 \cdot V_{u_id_j} + m_{u_k}
\Sigma^{u \star}_{ki} V_{kj} \right] L
 \right\} d_j H^+ \label{Sff2}~,
\end{eqnarray}
where $V$ is the $4 \times 4$ CKM matrix, $q=d$ or $u$ for down or up-quarks with $I_d=-1$ and $I_u=+1$, respectively,
and $R(L)=\frac{1}{2}\left(1+(-)\gamma_5\right)$.
Also, $\Sigma^d$ and $\Sigma^u$ are new mixing matrices where
all FCNC effects of the 4G2HDM are encoded. They are
obtained after diagonalizing the quark mass matrices and, therefore, depend on
the rotation (unitary) matrices of the right-handed down and up-quarks
$D_R$ and $U_R$, respectively. In particular, for ${\cal I} \equiv {\rm diag}\left(0,0,0,1\right)$
in Eq.~\ref{eq:LY4G}, we have (see \cite{ourpaper1}):$^{[2]}$\footnotetext[2]{Note that this
is in contrast to
``standard" frameworks such as the SM and the 2HDM's of types I and II,
where the right-handed mixing matrices $U_R$ and $D_R$ are non-physical,
being ``rotated away" in the diagonalization procedure of the quark masses.}
\begin{eqnarray}
\Sigma_{ij}^d = D_{R,4i}^\star D_{R,4j} ~,~ \Sigma_{ij}^u  =U_{R,4i}^\star U_{R,4j} ~.
\label{sigma}
\end{eqnarray}

The Yukawa structure and couplings defined by Eqs.~\ref{eq:LY4G}-\ref{sigma} is assumed
to be copied to the leptonic sector, see \cite{ourg-2}.
In the following sections \ref{sec3} and \ref{sec4},
for illustrative purposes (and without loss of generality), we will set
$\Sigma^{d,u} \to {\rm diag}\left(0,0,0,1\right)$ in both the quark and lepton sectors,
so that FCNC effects (in particular, between the 4th generation fermions
and the SM fermions) are ``turned off".
In fact, from the phenomenological point of view, it is sufficient
to assume that $\Sigma^{u}_{34,43} \to 0$ (i.e., forbidding
the decay $t^\prime \to t h$) and $V_{i4,4i} \to 0$ ($i=1,2,3$, thus forbidding
the decays $t^\prime \to d_i W$ and $b^\prime \to u_i W$ with $d_i=d,s,b$ and $u_i=u,c,t$)
in order to accommodate relatively light $t^\prime$ and $b^\prime$ with masses as low as 350 GeV,
since the existing stringent exclusion limits of $m_{t^\prime},m_{b^\prime} \:\raisebox{-0.5ex}{$\stackrel{\textstyle>}{\sim}$}\: 700$ GeV,
are based on searches that assume 100\% branching ratios of the 4th generation
quarks into one of the channels: $t^\prime \to th,tZ,d_i W$ and
$b^\prime \to Zb,u_iW$ \cite{pdg,1509.04261}.
We will, therefore, assume that
the dominant $t^\prime$ and $b^\prime$ decays are into one of the FC channels
$t^\prime \to u_ih$ and
$b^\prime \to d_i h$ ($u_i=u,c$ and $d_i=d,s,b$), due to small
FCNC entries in $\Sigma^{u,d}$ (which have no effect on the results presented in sections \ref{sec3} and \ref{sec4}),
in which case small off-diagonal CKM entries $V_{14,41}$ and/or $V_{24,42}$ are also allowed
as long as $BR(t^\prime \to d_i W),~BR(b^\prime \to u_iW) \:\raisebox{-0.5ex}{$\stackrel{\textstyle<}{\sim}$}\: 0.5$ \cite{1509.04261}.
Such flavor structures, may have interesting phenomenological implications,
as will be discussed in section \ref{sec5}.

The 2HDM scalar sector is parameterized by seven free parameters (after minimization
of the potential), which, in the so called
``physical basis", can be chosen as the four physical Higgs masses ($m_h,~m_H,~m_A,~m_{H^+}$),
the two angles
$\beta$ and $\alpha$ and one parameter from the scalar potential, which is needed
in order to specify the scalar couplings, in particular,
$hH^+H^-$ (which enters in the 1-loop $h \to \gamma \gamma$ decay), $HH^+H^-$
(which enters the 1-loop $H \to \gamma \gamma$ decay)
and $Hhh$ (required for the decay $H \to hh$).
In the physical basis, these
scalar couplings can be written at tree-level as
(see e.g., \cite{0408364}):
\begin{eqnarray}
\lambda_{Hhh}=-\frac{\cos(\alpha-\beta)}{2 v \sin 2\beta}
\left[ \sin 2 \alpha \left(m_h^2+2m_H^2 \right) -
\left( 3 \sin 2 \alpha - \sin 2 \beta \right)
\frac{m_{\ell h}^2}{s_\beta c_\beta} \right] \label{lam1} ~,
\end{eqnarray}
\begin{eqnarray}
\lambda_{hH^+H^-}=-\frac{1}{2 v \sin 2\beta}
\left[ \left( \cos(\alpha-3\beta)+3 \cos(\alpha+\beta) \right) m_h^2 -
4 \sin 2 \beta \sin(\alpha-\beta) m_{H^\pm}^2 -
4 \cos(\alpha+\beta) \frac{m_{\ell h}^2}{s_\beta c_\beta} \right] \label{lam2}  ~,
\end{eqnarray}
\begin{eqnarray}
\lambda_{HH^+H^-}=-\frac{1}{2 v \sin 2\beta}
\left[ \left( \sin(\alpha-3\beta)+3 \sin(\alpha+\beta) \right) m_H^2 +
4 \sin 2 \beta \cos(\alpha-\beta) m_{H^\pm}^2 -
4 \sin(\alpha+\beta) \frac{m_{\ell h}^2}{s_\beta c_\beta} \right] \label{lam3}  ~,
\end{eqnarray}
where $m_{\ell h}^2$ is a mass-like term,
$m_{\ell h}^2 \Phi_\ell^\dagger \Phi_h + h.c.$,
which softly breaks the above
$Z_2$-symmetry (i.e., $\Phi_{\ell}\to-\Phi_{\ell},~ \Phi_{h}\to+\Phi_{h}$),
and which can be used to specify the above tree-level
scalar couplings.

However, since
the working assumption of the 4G2HDM is that
the scalar sector may be strongly interacting at the near by few TeV scale,
the scalar potential is expected to be subject to significant renormalization and threshold effects.
Thus, the above scalar couplings are expected
to deviate from their tree-level values, depending
on the details of the UV completion and on the masses
of the heavy degrees of freedom of this model, see e.g.,
\cite{0408364,loop-cor}.
As an example, consider the 1-loop corrections to the $Hhh$ coupling $\lambda_{Hhh}$,
for $|\alpha| \to \pi/2$, in which case there is
no mixing between the light and heavy Higgs fields (see Eq.~\ref{Higgsangles}),
as
required in order to accommodate
the 750 GeV $\gamma \gamma$ excess in the 4G2HDM (see section \ref{sec4}).
In this limit, the Yukawa couplings of the 4th generation fermions
to the light Higgs state $h$ (i.e., $t^\prime t^\prime h$) vanish (see Eq.~\ref{Sff1} and Table \ref{tab4}) and
we find that
the dominant effect arises from the 1-loop triangle diagram
with the charged Higgs exchange in the loop, giving
a ``renormalized" $Hhh$ coupling $\bar\lambda_{Hhh} \equiv a_{Hhh} \lambda_{Hhh}$,
with:
\begin{eqnarray}
a_{Hhh} \approx 1+ \frac{m_{\ell h}^4}{m_H^2 v^2}
\frac{\left( 1-2c_\beta^2 \frac{m_{H^+}^2}{m_{\ell h}^2} \right)
\left(1+c_\beta^2 \frac{m_{H}^2}{m_{\ell h}^2} - 2s_\beta^2 \frac{m_{H^+}^2}{m_{\ell h}^2}
\right)}{2 \pi^2 (\sin2\beta)^2} I\left(m_h,m_H,m_{H^+} \right)~,
\end{eqnarray}
where $I\left(m_h,m_H,m_{H^+} \right)$ is the charged Higgs triangle loop integral, given by:
\begin{eqnarray}
I\left(m_h,m_H,m_{H^+} \right) = - \int_0^1 dx \int_0^{1-x} dy ~
\frac{1}{ (x+y) (x+y-1) m_h^2 - xy m_H^2 + m_{H^+}^2  } ~.
\end{eqnarray}
In particular, one roughly finds $|a_{Hhh}| \in \left\{0, 2\right\}$ when
$m_{H^+} \in \left\{500~{\rm GeV}, 1~{\rm TeV} \right\}$ and with
$m_H =750$ GeV, $m_h =125$ GeV and $m_{\ell h} \sim {\cal O}(1~{\rm TeV})$.
For example, $a_{Hhh} \sim -0.15$ for $m_{H^+} = m_H = 750$ GeV and
$m_{\ell h} =1.2$ TeV. In what follows we will, therefore,
define the ``renormalized" scalar couplings as: $\bar\lambda_i \equiv a_i \lambda_i$,
where $\lambda_i$ ($i=Hhh,~ hH^+H^-,~HH^+H^-$) are
the corresponding tree-level couplings in Eqs.~\ref{lam1}-\ref{lam3}, and
$a_i$ will be treated as free-parameters in the fit that will be varied in the range
$|a_i| \in \left\{0, 2\right\}$.

\section{The 125 GeV Higgs signals and PEWD \label{sec3}}

The measured signals of the 125 GeV Higgs particle, which in the 4G2HDM
is the light Higgs $h$, and PEWD impose stringent constraints
on the free parameter space of the 4G2HDM.
For the 125 GeV Higgs signals we use the measured values of the
``signal strength" parameters, which are defined as the ratio between the measured
rates and their SM expectation.
In particular, for a specific production and decay
channel $i \to h \to f$, the signal strength is defined as:
\begin{eqnarray}
\mu_{i}^f \equiv \mu_i \cdot \mu^f ~,
\end{eqnarray}
with
\begin{eqnarray}
\mu_i = \frac{\sigma(i \to h)}{\sigma(i \to h)_{SM}} = k_i^2~,~
\mu^f = \frac{BR(h \to f)}{BR(h \to f)_{SM}} = \frac{k_f^2}{R^T} ~,
\end{eqnarray}
where $k_j$ is the 4G2HDM coupling involved in $j \to h$ or $h \to j$ production or decay processes, normalized by its SM value, and $R^T$
is the ratio between the total width of $h$ in the 4G2HDM and the
total width of the SM 125 GeV Higgs. In particular,
\begin{eqnarray}
k_j \equiv \frac{k_j^{4G2HDM}}{k_j^{SM}} ~,~
R^T \equiv \frac{\Gamma_{h_{4G2HDM}}^{Total}}{\Gamma_{h_{SM}}^{Total}}~,
\end{eqnarray}
so that $\mu_i^f = k_i^2 k_f^2 / R^T$.

In Table \ref{tab1} we list the latest combined ATLAS and CMS six parameter fit from RUN1
\cite{ATLAS-CMS-125res}, of the measured
values for $\mu_{gg}^{\gamma \gamma},~\mu_{gg}^{WW^\star},
~\mu_{gg}^{ZZ^\star},~\mu_{gg}^{bb},~\mu_{gg}^{\tau \tau}$
and $\mu_V/\mu_{gg}$, where $\mu_V$ stands for Higgs
production via vector-boson fusion (VBF) or in association with a
vector-boson (VH).$^{[3]}$\footnotetext[3]{We neglect Higgs production
via $pp \to tth$ which, although included in the fit, is
2-3 orders of magnitudes smaller than the gluon-fusion channel}.
We also write in Table \ref{tab1} the model predictions for the various signal strengths in terms
of the normalized couplings defined above.

\begin{table}[htb]
\begin{center}
\begin{tabular}{c||c|c|}
 & measured value & model prediction / couplngs \\
\hline \hline
 $\mu_{gg}^{\gamma \gamma} $ & $1.13^{+0.24}_{- 0.21}$  & $k_g^2  k_\gamma^2 /R^T $ \\
\hline
$\mu_{gg}^{ZZ^\star}  $ & $1.29^{+0.29}_{- 0.25}$ & $k_g^2 k_V^2 /R^T$ \\
\hline
$\mu_{gg}^{WW^\star} $ & $1.08^{+0.22}_{- 0.19}$ & $k_g^2  k_V^2 /R^T$ \\
\hline
$\mu_{gg}^{bb} $ & $0.65^{+0.37}_{- 0.28}$ & $k_g^2 k_b^2/R^T$ \\
\hline
$\mu_{gg}^{\tau \tau} $ & $1.07^{+0.35}_{- 0.28}$ & $k_g^2  k_\tau^2 /R^T$ \\
\hline
$\mu_V/\mu_{gg} = $ & $1.06^{+0.35}_{- 0.27}$ & $k_V^2 / k_g^2$ \\
\hline
\end{tabular}
\caption{Measured
values \cite{ATLAS-CMS-125res} and model predictions in terms of normalized couplings (see text)
of the various production and decay channels for the 125 GeV Higgs,
using the signal strength prescription.
Note that while $k_V,k_b$ and $k_\tau$ are ratios of tree-level
couplings, $k_g$ and $k_\gamma$ are the normalized (with respect to the SM)
1-loop 4G2HDM couplings $hgg$ and $h\gamma \gamma$, respectively, calculated
using the formula in \cite{HHG}.
Also, in our 4G2HDM $k_W=k_Z=k_V$.}
\label{tab1}
\end{center}
\end{table}

For the PEWD constraints on the 4G2HDM, we update our study in \cite{ourpaper1}.
In particular, the effects of any new physics can be divided into those
which do and which do not couple directly
to the ordinary SM fermions.
For the former, the leading effect in the 4G2HDM comes from the decay
$Z \to b \bar b$, which is mainly sensitive to the
$H^+ t^\prime b$ and $W^+ t^\prime b$ couplings through one-loop exchanges of $H^+$ and $W^+$, as was analyzed in detail in \cite{ourpaper1}.
These contributions to $Z \to b \bar b$ are, however, absent in the currently studied
versions of the 4G2HDM, since our working assumption here
is that $V_{t^\prime b} \to 0$ and $\Sigma^{d,u} \to {\rm diag}\left(0,0,0,1\right)$,
so that the $H^+ t^\prime b$ and $W^+ t^\prime b$ vertices vanish
or are negligibly small (see previous section).

The effects which do not involve direct couplings to the ordinary fermions,
can be analyzed in the formalism of the oblique parameters S,T and U
\cite{peskin}. The contribution of a 2HDM with a 4th generation of chiral fermions
to the oblique parameters were studied in \cite{ourpaper1}.
This includes the pure 1-loop Higgs exchanges
to the gauge-bosons 2-point functions and the 1-loop exchanges of
$t^\prime$ and $b^\prime$ which shift the T parameter
and which involve the new SM4-like diagonal coupling
$W t^\prime b^\prime$ (here also the contributions involving the
off-diagonal couplings $W t^\prime b$ and $W t b^\prime$ are absent
since we assume $V_{t^\prime b},~ V_{t b^\prime} \to 0$, see also \cite{deltaT}).
These are calculated with respect
to the SM values and are bounded by a global fit to PEWD \cite{gfitter}:
\begin{eqnarray}
\Delta S &=& S - S_{SM} = 0.06 \pm 0.09 ~, \nonumber \\
\Delta T &=& T - T_{SM} = 0.1 \pm 0.07 \label{SandT}~,
\end{eqnarray}
with a correlation coefficient of $\rho = +0.91$.
These values are obtained for $\Delta U=0$
(the $U$ parameter is often set to zero since
it can be neglected in most new physics models and, in particular
in our 4G2HDM) and
with the SM reference values
$M_{H,{\rm ref}}=125$ GeV and $m_{t,{\rm ref}}=173$ GeV.
We, thus,
consider below the constraints from the 2-dimensional ellipse in the $S-T$ plane
which, for a given confidence level (CL), is defined by:
\begin{widetext}
\begin{eqnarray}
\left(
\begin{array}{c} S - S_{exp} \\ T - T_{exp}  \end{array}
\right)^T
\left(
\begin{array}{cc} \sigma_S^2 & \sigma_S \sigma_T \rho \\
\sigma_S \sigma_T \rho & \sigma_T^2 \end{array}
\right)
\left(
\begin{array}{c} S - S_{exp} \\ T - T_{exp}  \end{array}
\right)
= - 2 {\rm ln}\left( 1 - CL \right) \label{ST2}~,
\end{eqnarray}
\end{widetext}
where $S_{exp} = 0.06$ and $T_{exp} = 0.1$ are the best fitted (central)
values, $\sigma_S = 0.09, \sigma_T = 0.07$
are the corresponding standard deviations and $\rho=0.91$
is the (strong) correlation factor between S and T.

We thus perform a random (``blind") scan of the
relevant parameter space, imposing compatibility at 95\% CL
of the 4G2HDM with the measured 125 GeV Higgs signals
listed above and with the best fitted values of $S$ and $T$
using Eqs.~\ref{SandT} and \ref{ST2}. In particular, we fix $m_H=750$ GeV
(for compatibility with the recent 750 GeV $\gamma \gamma$ signal, see next section) and scan
the rest of the parameters over the following ranges:
\begin{eqnarray}
\alpha \in \left[ - \frac{\pi}{2},\frac{\pi}{2} \right] ~,~
\tan\beta \in \left[ 0.4 , 10 \right]~,~ a_i\in \left[ -2,2 \right] ~
(i=hH^+H^-,HH^+H^-,Hhh) ~, \nonumber
\end{eqnarray}
\begin{eqnarray}
m_{\ell h}^2 \in \left[ - \left(2~ {\rm TeV} \right)^2,\left(2~ {\rm TeV} \right)^2 \right] ~,~
m_{A,H^+} \in \left[ 300~ {\rm GeV} ,1.5~ {\rm TeV} \right]  ~, \nonumber
\end{eqnarray}
\begin{eqnarray}
m_{t^\prime,b^\prime} \in \left[ 350~{\rm GeV} , 500~{\rm GeV} \right] ~,~
m_{\nu^\prime,\tau^\prime} \in \left[ 200~{\rm GeV} , 1200~{\rm GeV} \right] ~.
\end{eqnarray}

\begin{figure}
\begin{center}
\includegraphics[scale=0.27]{SandT_case1.eps}
\includegraphics[scale=0.27]{alpha_vs_tb_case1.eps}
\includegraphics[scale=0.27]{deltam_case1.eps}
\includegraphics[scale=0.27]{signal_strength_case1.eps}
\includegraphics[scale=0.27]{SandT_case3.eps}
\includegraphics[scale=0.27]{alpha_vs_tb_case3.eps}
\includegraphics[scale=0.27]{deltam_case3.eps}
\includegraphics[scale=0.27]{signal_strength_case3.eps}
\end{center}
\caption{The distribution of the 4G2HDM parameter space that is compatible
with the 125 GeV signals and PEWD. From left to right: in the $S -T$ plane (yellow, pink and green ellipses correspond
to the 68\%, 95\% and 99\% CL allowed contours, respectively), in
the $\tan\beta - \sin\alpha$ plane, in the
$\Delta m_{\ell^\prime} - \Delta m_{q^\prime}$ plane,
where $\Delta m_{\ell^\prime} \equiv m_{\nu^\prime} - m_{\tau^\prime}$ and $\Delta m_{q^\prime} \equiv m_{t^\prime} - m_{b^\prime}$
and the corresponding 125 GeV signal
strengths (on right). Case 1 in the upper row, case 2 in the middle row and case 3 in the lower row,
see text.
\label{fig1}}
\end{figure}

We find two types of possible 4G2HDM ``solutions":
\begin{description}
\item{case 1:} $\tan\beta \leq 0.5$, $\sin\alpha \to -1$ and $m_{\ell h}^2 > 0$.
\item{case 2:} $\tan\beta \geq 2$, $\sin\alpha \sim 0.1 - 0.45$ and any $m_{\ell h}^2$ in the entire range scanned.
\end{description}

In both cases above, $m_A,~m_{H^+}$ and the 4th generation fermion masses
can have values spanning over the entire scan ranges.
In Fig.~\ref{fig1} we plot the resulting distributions of the relevant parameter space
in the $S -T$, $\tan\beta - \sin\alpha$ and
$\Delta m_{\ell^\prime} - \Delta m_{q^\prime}$ planes, where
$\Delta m_{\ell^\prime} \equiv m_{\nu^\prime} - m_{\tau^\prime}$ and
$\Delta m_{q^\prime} \equiv m_{t^\prime} - m_{b^\prime}$. We
also show in Fig.~\ref{fig1} the resulting predicted 125 GeV Higgs signal
strengths for the two cases above, which, as can seen, have different characteristics.

We next discuss the compatibility of the above two 4G2HDM solutions with the recently observed
750 GeV $\gamma \gamma$ excess.

\section{The 4G2HDM and the 750 GeV $\gamma \gamma$ resonance \label{sec4}}

We search here for the portion of parameter space of the two 4G2HDM cases
found in the previous section, that survive once the 4G2HDM is also required to accommodate the 750 GeV
$\gamma \gamma$ excess, which is being
interpreted here as the decay of one or both of the heavy neutral Higgs (i.e.,
assumed to have masses $\sim 750$ GeV) $H \to \gamma \gamma$ and/or $A \to \gamma \gamma$.

Given the exploratory nature of our study,
we will simplify our analysis at this point, assuming that the scalar spectrum have the
characteristics
of the so-called decoupling limit (see e.g., \cite{decouplinglimit}). In particular,
we assume that it is
split into 2 typical scales:
$m_{light} \sim 125$ GeV, corresponding to the observed light Higgs
and $m_{heavy} \sim 750$ GeV around which the three heavy Higgs masses lie,
i.e., $m_H,m_A,m_{H^+} \sim 750$ GeV.
Even though we find a wider range of allowed masses for the non-resonant heavy scalar states
(i.e., for $m_A$ and $m_{H^+}$, see below)
that can accommodate the 750 GeV signal,
the choice $m_H,~m_A,m_{H^+} \sim 750$ GeV will suffice for
conveying our point: that the
750 GeV resonance in the $\gamma\gamma$ channel can be accommodated by
one of the heavy scalars of the 4G2HDM without any conflict with other existing relevant data.
Indeed, if this measurement will be eventually confirmed, then it will be instructive
to study the 4G2HDM within a wider range of the relevant parameter space.

We, thus, re-scan the 4G2HDM parameter space corresponding to two 4G2HDM cases found in
the previous section, where now $m_H$, $m_A$ and $m_{H^+}$ are
varied within a 30 GeV mass range around 750 GeV, i.e., $m_{H,A,H^+} \in 750 \pm 30$ GeV.
The scan is performed with the following additional ``filters"/requirements
(i.e., in addition to the requirement of compatibility with PEWD and with the measured
125 GeV Higgs signals, as outlined in the previous section):
\begin{itemize}
\item Reproducing the 750 GeV $\gamma \gamma$ excess within the range
$3 ~{\rm fb} < \sigma(pp \to H/A \to \gamma \gamma) < 13~{\rm fb}$. We find that
the (by far) dominant $H$ and/or $A$ production mechanism is the gluon-fusion
one $gg \to H/A$, so that all the relevant
cross-sections $\sigma(pp \to H/A \to f)$
are calculated in the narrow width approximation via:
\begin{eqnarray}
\sigma(pp \to H/A \to f) = \frac{C_{gg}}{s m_{H/A}}
\Gamma(H/A \to gg) BR(H/A\to f) ~,
\end{eqnarray}
where $\sqrt{s} =8$ or $13$ TeV and $C_{gg}$ is the gluon luminosity:
\begin{eqnarray}
C_{gg} = \frac{\pi^2}{8} \int_{m_{H/A}^2/s}^1 \frac{dx}{x} g(x)
g\left( \frac{m_{H/A}^2}{sx} \right) ~,
\end{eqnarray}
giving $C_{gg} \sim 2140(175)$ at $\sqrt{s} =13(8)$ TeV, see \cite{gluonPDF}.

\item The resonating scalar which produces the 750 GeV $\gamma \gamma$ excess is required
to have a width smaller than 45 GeV, i.e., $\Gamma_{H/A} < 45$ GeV.

\item We impose the existing experimental bounds
on the production and decays of the
heavy neutral scalars $H$ and $A$, as obtained at the 8 and 13 TeV LHC runs (in particular when applied to
$m_H,m_A \sim 750$ GeV) in all other channels which are
relevant to our study:
$pp \to W^+W^-,~ZZ,~t \bar t,~\tau \tau,~b \bar b,~hh,~hZ$.
In particular, we use the 95\% CL bounds in Table \ref{tab2}
quoted in \cite{1605.09401}.
\end{itemize}

\begin{table}[htb]
\begin{center}
\begin{tabular}{c||c|c|}
 final state & $\sigma$ at $\sqrt{s}=8$ TeV & $\sigma$ at $\sqrt{s}=13$ TeV \\
\hline \hline
 $pp \to H \to W^+ W^- $ & $< 40 $ fb & $< 300$ fb\\
\hline
 $pp \to H \to ZZ $ & $< 12 $ fb & $< 200$ fb\\
\hline
 $pp \to H \to hh $ & $< 39 $ fb & $< 120$ fb\\
\hline
$pp \to A \to hZ $ & $< 19 $ fb & $< 116$ fb\\
\hline
$pp \to H/A \to t \bar t $ & $< 450 $ fb &  \\
\hline
$pp \to H/A \to b \bar b $ & $< 1 $ pb &  \\
\hline
$pp \to H/A \to j j $ & $< 2.5 $ pb &  \\
\hline
$pp \to H/A \to \tau \tau $ & $< 12 $ fb & $< 60$ fb \\
\hline
\end{tabular}
\caption{Upper bounds at 95\% CL on $\sigma(pp \to S \to f)$
for various final states $f$, produced through a narrow resonance with
$m_S \sim 750$ GeV and $\Gamma_S/m_S \sim {\cal O}(10^{-2})$,
as applied to our scan with $S = H,A$.
The bound on $\sigma( pp \to H/A \to jj)$ is relevant for $j = {\rm gluon}$.
Table taken from \cite{1605.09401}.}
\label{tab2}
\end{center}
\end{table}

Applying the above filters, we find that:
\begin{enumerate}
\item Only the CP-even scalar state $H$ (with $m_H =750$ GeV),
can accommodate the 750 GeV $\gamma \gamma$ resonance, since
$\sigma(pp \to A \to \gamma \gamma) \:\raisebox{-0.5ex}{$\stackrel{\textstyle<}{\sim}$}\: {\cal O}(0.01)$ fb, which is 2-3 orders of
magnitudes smaller than the measured $\gamma \gamma$ excess, see also Table \ref{tab4}.
\item Only a ``shrinked" version of
the 4G2HDM case 1 survives out of the two cases that were found to be compatible with PEWD and
the 125 GeV light Higgs signals. In particular,
the surviving 4G2HDM models have (see Fig.~\ref{fig2}): $\tan\beta \leq 0.5$, $\alpha \to -\pi/2$
and $m_{\ell h} > 600$ GeV, having some correlation with the renormalization factors of the scalar couplings
$a_i = \bar\lambda_i/\lambda_i$, $i=Hhh,~ hH^+H^-,~HH^+H^-$.
\item The resulting heavy fermions mass ranges are narrowed to:
$350 ~ {\rm GeV} \:\raisebox{-0.5ex}{$\stackrel{\textstyle<}{\sim}$}\: m_{t^\prime},m_{b^\prime} \:\raisebox{-0.5ex}{$\stackrel{\textstyle<}{\sim}$}\: 390 ~ {\rm GeV}$, where the lower limit
is from direct searches (see section \ref{sec2}),
and $900 ~ {\rm GeV} \:\raisebox{-0.5ex}{$\stackrel{\textstyle<}{\sim}$}\: m_{\nu^\prime},m_{\tau^\prime} \:\raisebox{-0.5ex}{$\stackrel{\textstyle<}{\sim}$}\: 1200 ~ {\rm GeV}$,
where the upper limit is a rough estimate of the perturbativity bound on heavy chiral
leptons.
\end{enumerate}

In Fig.~\ref{fig2} we show three
scatter plots of the resulting 4G2HDM parameter space, corresponding to
the mass spectrum of the heavy fermions, the correlation between the soft breaking mass
parameter $m_{\ell h}$ and the renormalization factor of the scalar couplings
$a_i = \bar\lambda_i/\lambda_i$, $i=Hhh,~ hH^+H^-,~HH^+H^-$, and the resulting
allowed ranges of the 125 GeV light Higgs signal strengths in all the measured channels.
We see that, while $|m_{t^\prime} - m_{b^\prime}| \:\raisebox{-0.5ex}{$\stackrel{\textstyle<}{\sim}$}\: 30$ GeV,
the mass splitting of the heavy leptons is typically $|m_{\nu^\prime} - m_{\tau^\prime}| \:\raisebox{-0.5ex}{$\stackrel{\textstyle>}{\sim}$}\: m_W$.
We also see that smaller values of $m_{\ell h}$ typically require larger values of the
renormalization factors of the scalar vertices $a_i$, e.g., $a_{Hhh} \sim 1$
for $m_{\ell h} \sim 700$ GeV.

\begin{figure}
\begin{center}
\includegraphics[scale=0.37]{Fig2_deltam.eps}
\includegraphics[scale=0.37]{fig2_ai_vs_mlh.eps}
\includegraphics[scale=0.37]{fig2_125_signals.eps}
\end{center}
\caption{Scatter plots of the 4G2HDM parameter space that is compatible
with the 125 GeV signals, with PEWD, with
$\sigma(pp \to H\to \gamma \gamma) = 3-13$ fb, with $\Gamma_H \leq 45$ GeV and
with all 8 and 13 TeV LHC bounds on the cross-section
$\sigma(pp \to H/A \to f)$ in all final states $f$ relevant to the $H$ and $A$ decays,
see Table \ref{tab2}. The scatter plots are given
for the mass splitting spectrum of the heavy fermions (left),
the correlation between the soft breaking mass
parameter $m_{\ell h}$ and the renormalization factor of the scalar couplings
$a_i = \bar\lambda_i/\lambda_i$, $i=Hhh,~ hH^+H^-,~HH^+H^-$ (middle), and the resulting
allowed ranges of the 125 GeV light Higgs signal strengths in all the measured channels (right).
\label{fig2}}
\end{figure}

It is interesting to note that the resulting mass spectrum
of the heavy chiral quarks, which is required to accommodate the 750 GeV
$\gamma \gamma$ resonance, is rather narrow and
roughly centered around $m_H /2$, i.e.,
$m_{t^\prime},m_{b^\prime} \sim 350 - 390 ~ {\rm GeV}$.
This may hint back to the possibility that the
the heavy scalars are composites primarily
of the heavy chiral quarks, in which
case the 4G2HDM might indeed be interpreted
as a low energy effective framework for some TeV-scale strongly interacting
theory. Such an effective low energy 2HDM, with features similar
to the 4G2HDM discussed here,
was introduced in \cite{ourhybrid}, where it was shown that,
using the Nambu-Jona-Lasinio (NJL) mechanism \cite{Nambu}, it is possible to construct an
effective sub-TeV 2HDM hybrid framework, in which the 125 GeV light Higgs is mostly
a fundamental scalar, while the heavy Higgs states are components of
a composite field of the form
$\Phi_h \sim g_{t^\prime}^\star < \bar Q_L^{\prime c} (i \tau_2) t^{\prime c}_R > + g_{b^\prime} < \bar Q_L^\prime b^\prime_R >$, which is responsible
for EW symmetry breaking and for the dynamical mass generation of the heavy
quarks.$^{[4]}$\footnotetext[4]{Another interesting framework which entertains the idea that heavy chiral quarks
may form the 750 GeV composite was recently suggested in \cite{1602.05539}.}

\section{Phenomenology of the 4G2HDM \label{sec5}}

Inspired by the indications of the 750 GeV $\gamma \gamma$ resonance
and following the analysis of the previous section,
we briefly consider here
some of the distinct phenomenological consequences of the 4G2HDM
with characteristics similar to those
required to accommodate such a heavy scalar resonance.

In particular, we will assume below that $\tan\beta \sim 0.5$
and $\sin\alpha \sim -1$, in which case the light 125 GeV Higgs of the 4G2HDM, $h$, does not
couple to $f^\prime f^\prime$, while the heavy CP-even Higgs, $H$,
does not couple to a pair of SM fermions (see Eqs.~\ref{Sff1}-\ref{Sff2} and Table \ref{tab3}).
Also, the 4th generation heavy fermions are assumed to have masses in the ranges
$350 ~ {\rm GeV} \:\raisebox{-0.5ex}{$\stackrel{\textstyle<}{\sim}$}\: m_{t^\prime},m_{b^\prime} \:\raisebox{-0.5ex}{$\stackrel{\textstyle<}{\sim}$}\: 400 ~ {\rm GeV}$
and $900 ~ {\rm GeV} \:\raisebox{-0.5ex}{$\stackrel{\textstyle<}{\sim}$}\: m_{\nu^\prime},m_{\tau^\prime} \:\raisebox{-0.5ex}{$\stackrel{\textstyle<}{\sim}$}\: 1200 ~ {\rm GeV}$,
and the dominant decay channels of the heavy quarks are
$t^\prime \to uh$ ($u=u,c$) and $b^\prime \to dh$ ($d=d,s,b$), with
corresponding branching ratios $ \:\raisebox{-0.5ex}{$\stackrel{\textstyle>}{\sim}$}\: 0.5$,
due to small off diagonal-entries $\Sigma^u_{4i}$ ($i=1,2$) and/or
$\Sigma^d_{4i}$ ($i=1,2,3$)
(see Table \ref{tab3} and discussion in section \ref{sec2}).

\begin{table}[htb]
\begin{center}
\begin{tabular}{|c||c|c|c|}
 & \multicolumn{3}{c|}{Yukawa couplings in the 4G2HDM with $\sin\alpha \sim -1$} \\
\hline
  &  $v \cdot y(\bar f f)$
  & $v \cdot y(\bar f^\prime f^\prime)$
 & $v \cdot y(\bar f_i f_{j})$ ($i, j = 1-4, i\neq j$)  \\
\hline \hline
 $h$ & $-\frac{m_f}{\cos\beta}$ & 0 &  $\frac{\Sigma^f_{ij}}{\cos\beta} (m_{f_i} R + m_{f_j} L)$ \\
\hline
 $H$ & 0 & $\frac{m_f}{\sin\beta}$ &  $ \frac{\Sigma^f_{ij} }{\sin\beta} (m_{f_i} R + m_{f_j} L)$ \\
\hline
 $A$ & $-i I_f m_f \tan\beta$  & $i I_f m_{f^\prime} \cot\beta$ &  $i I_f \frac{\Sigma^f_{ij}}{\sin\beta \cos\beta} (m_{f_i} R - m_{f_j} L)$ \\
  \hline
\end{tabular}
\caption{Yukawa couplings of the neutral Higgs particles in the 4G2HDM with $\sin\alpha \to -1$
and assuming $\Sigma^f_{ij} \ll \Sigma^f_{44} =1$ for
$ij \neq 44$, see section \ref{sec2}. In the first column
$f$ is a SM fermion of the 1st-3rd generations, while in the second column
$f^\prime$ stands for a 4th generation
fermion. In the 3rd column $f_i$ correspond to any fermion of the $i$th generation. Also, $I_f = 1(-1)$
for up(down) type fermions.}
\label{tab3}
\end{center}
\end{table}

In Table \ref{tab4} we list three benchmark points (BMP1,BMP2,BMP3)
which have some distinct characteristics and which are compatible with PEWD,
with the 125 GeV Higgs signals, with the 750 GeV $\gamma \gamma$ signal
and with the LHC bounds on all relevant 750 GeV Higgs resonance channels
$pp \to H/A \to f$ given in Table \ref{tab2}.
For definiteness, we have generated the benchmark points for the case of
$m_H = 750 $ GeV and $m_A,m_{H^+} \sim m_H \pm 50$ GeV, but the discussion below has a
more general scope, i.e., with regard to some of the possible
phenomenological signatures of the 4G2HDM associated with the TeV-scale
heavy scalars of the model and independent of whether the 750 GeV
$\gamma \gamma$ resonance is confirmed or not.
The three benchmark points include cases where the 750 GeV Higgs total width ranges from
a few GeV to $\sim 45$ GeV, having a resonance cross-section to $\gamma \gamma$ between 4-12 fb.
They also correspond to cases where $BR(H/A \to \bar q^\prime q^\prime) \sim 1$ and
$BR(H^+ \to \bar q^\prime q^\prime) \sim 1$.

\begin{table}[htb]
\begin{center}
\begin{tabular}{|c||c|c|c|}
\hline
  & BMP1 & BMP2 & BMP3  \\
\hline \hline
 $m_{t^\prime},m_{b^\prime}, m_{H^+}, m_A$ [GeV] & $352,382,709,780$ & $384,373,795,778$ & $368,369,691,731$   \\
\hline
 $H$ total width, $\Gamma_H$ [GeV] & 43 & 4 & 17   \\
\hline
 $\sigma(pp \to H/A \to \gamma \gamma)$ [fb] & $4/0.004$ & $12/0.006$ & $8/0.005$    \\
\hline
 $BR(H \to \bar t^\prime t^\prime, \bar b^\prime b^\prime, \bar t t, hh,gg)$ & $0.94,0,{\cal O}(10^{-6}),{\cal O}(10^{-4}),0.06$ &
 $0,0.36,0.04,0.007,0.64$& $0.47,0.38,{\cal O}(10^{-6}),{\cal O}(10^{-4}),0.14$  \\
\hline
$BR(A \to \bar t^\prime t^\prime, \bar b^\prime b^\prime, \bar t t, hZ,gg)$ & $0.61,0.33,0.015,0.04,{\cal O}(10^{-4})$ & $0.33,0.61,0.016,0.05,0.004$ & $0,0,0.29,0.71,{\cal O}(10^{-4})$   \\
\hline
 $\sigma(pp \to H \to \bar t^\prime t^\prime, \bar b^\prime b^\prime, \bar t t, hh)$ [fb] &
 $15000,0,0.015,5$
  & $0,4000,0.65,109$ & $7500,6000,0.02,9$  \\
\hline
 $\sigma(pp \to A \to \bar t^\prime t^\prime, \bar b^\prime b^\prime, \bar t t, hZ)$ [fb] &
 $160,87,19,52$
  & $90,164,21,57$
   & $0,0,38,91$   \\
\hline
 $BR(H^+ \to t^\prime \bar b^\prime, t \bar b ,W^+h)$ & $0,0.31,0.69$ & $0.9,0.03,0.07$ & $0,0.32,0.68$    \\
\hline
\end{tabular}
\caption{Benchmark points
with some distinct characteristics, which are consistent with PEWD,
with the 125 GeV Higgs signals, with the 750 GeV $\gamma \gamma$ signal
and with the LHC bounds on all relevant 750 GeV Higgs resonant channels
$pp \to H/A \to f$ given in Table \ref{tab2}.}
\label{tab4}
\end{center}
\end{table}

In particular, if $m_H,m_A > m_{q^\prime}/2$, then $H/A \to \bar q^\prime q^\prime$
is open and typically dominates, having a branching ratio of ${\cal O}(1)$ (see Table \ref{tab4}).
In that case, we find that within the 4G2HDM parameter space discussed here,
the corresponding resonance cross-sections
for $\bar q^\prime q^\prime$ production at the 13 TeV LHC are typically
$\sigma(pp \to H \to q^\prime q^\prime) \sim {\cal O}(10)$ [pb] and
$\sigma(pp \to A \to q^\prime q^\prime) \sim {\cal O}(0.1)$ [pb],
(both $H$ and $A$ produced through
gluon-fusion $gg \to H/A$), so that in the case of $H \to q^\prime q^\prime$ (see Table \ref{tab4}), this is
about an order of magnitude larger than the QCD (continuum) $\bar q^\prime q^\prime$ production rate.
Therefore, if the 750 GeV $\gamma \gamma$ resonance persists,
one should also expect an observable resonance signal at least in the
$H \to \bar q^\prime q^\prime$ channel.

Let us, therefore, briefly investigate the signal $H \to \bar q^\prime q^\prime$
under more general grounds, i.e., when $m_H > m_{q^\prime}/2$ but not necessarily
$m_H \sim 750$ GeV.
For example, in the case of $H \to \bar t^\prime t^\prime$,
the $t^\prime$ will further decay either via the FC channels $t^\prime \to uh$ ($u=u$ or $c$) or
via the 3-body decay $t^\prime \to b^\prime W \to dhW$ ($d=d,s,b$), where $b^\prime W$ are either off-shell
or on-shell (i.e., when $m_{t^\prime} > m_{b^\prime}+m_W$, see Fig.~\ref{fig1}).
If the former case (i.e., $t^\prime \to uh$) dominates, then the resulting resonance signal should be searched for
in $pp \to \bar t^\prime t^\prime \to (jh)_{t^\prime}(jh)_{t^\prime}$ ($j$ is a light jet),
while if the 3-body $t^\prime$ decay dominates then
$pp \to \bar t^\prime t^\prime \to (jhW^+)_{t^\prime}(jhW^-)_{t^\prime}$.
In either case, the SM-like light Higgs ($h$) further decays
into $b \bar b$ or $WW$ with SM rates, giving rise to resonance signatures
of the form $pp \to (nj+mb+\ell W)_H$, with
$(n,m,\ell)=(2,4,0),(2,0,4),(2,2,2),(2,4,2),(2,2,4),(2,0,6),(0,2,6),(0,4,4),(0,6,2)$
and with unique kinematic features
that distinguishes them from more conventional signatures.
Similar signals are also expected for $H \to \bar b^\prime b^\prime$.
We recognize that these type of signals are very challenging and may require new strategies,
in particular, for reconstructing the parent $q^\prime$'s in such a high jet-multiplicity environment.

The decay pattern of the charged Higgs may also change in the 4G2HDM,
in particular for the case when $m_{H^+} > m_{t^\prime} + m_{b^\prime}$,
for which the decay of  $H^+$ into a pair of heavy 4th generation fermions can dominate (see BMP1 in Table \ref{tab4}).
In particular, taking $m_{t^\prime} \sim m_{b^\prime} \equiv m_{q^\prime}$
and assuming that $H^+$ is sufficiently heavier than
$2m_{q^\prime}$, so that we can ignore corrections of
${\cal O}(4m_{q^\prime}^2/m_{H^+}^2)$ in the
phase-space factors, we have in the 4G2HDM:
\begin{eqnarray}
R_{t^\prime b^\prime/tb} &\equiv& \frac{\Gamma(H^+ \to t^\prime b^\prime)}{\Gamma(H^+ \to t b)}
\sim 2 \frac{m_{q^\prime}^2}{m_t^2} \cot^4\beta ~, \\
R_{t^\prime b^\prime/Wh} &\equiv& \frac{\Gamma(H^+ \to t^\prime b^\prime)}{\Gamma(H^+ \to Wh)}
\sim 12 \frac{m_{q^\prime}^2}{m_{H^+}^2} \left(\frac{\cot\beta}{\cos(\beta -\alpha)}\right)^2 ~.
\end{eqnarray}

Thus, for $\alpha \sim - \pi/2$, $\tan\beta \sim 0.5$ (i.e.,
$\cos(\beta - \alpha) \sim -0.45$), $m_{q^\prime} \sim 350$ GeV
(i.e., values of the 4G2HDM parameter space that can accommodate the 750 GeV $\gamma \gamma$ signal)
and taking $m_{H^+} \sim {\cal O}(1)$ TeV, we obtain: $R_{t^\prime b^\prime/tb} \sim {\cal O}(100)$
and $R_{t^\prime b^\prime/Wh} \sim {\cal O}(10)$, in which case
$BR(H^+ \to t^\prime b^\prime) \sim 1$ (e.g., as in the case of BMP2), leading to some interesting signatures
of the heavy charged Higgs at the LHC. In particular, the dominant production channels
of $H^+$ at the LHC are $gg/gb \to H^+ b \bar t, H^+ W^-/ H^+ \bar t$,
with a typical cross-section of $\sim 100$ fb when $\tan\beta \sim 1$ \cite{Hplusprod}.
The subsequent $H^+$ decay to a pair of 4th generation heavy fermions with
$BR(H^+ \to t^\prime \bar b^\prime) \sim 1$ will, thus, lead
to new $H^+$ signals, e.g.,
$pp \to t (t^\prime b^\prime)_{H^+} \to (b W)_t (jh)_{t^\prime} (jh)_{b^\prime}$, again
with the typical 4G2HDM heavy fermion high jet-multiplicity
signatures of the form $pp \to nj+mb+\ell W$.
This is in contrast to ``standard" 2HDM frameworks where the heavy charged Higgs
will dominantly decay to $Wh$ and/or $tb$ (see BMP1 and BMP3), leading to a lower multiplicity
of jets in the final state.

As noted earlier, a wider range of solutions exist (which are not being discussed here) to all data
and filters mentioned above (i.e., including the 750 GeV $\gamma \gamma$ resonance),
in which lighter pseudoscalar
$A$ and charged Higgs $H^{+}$ are allowed, with masses as low as $300$ GeV.
In such 4G2HDM scenarios, the heavy 4th generation quarks (and leptons) can
have substantial decay rates in channels involving also the heavy Higgs
species, i.e., $t^\prime \to H^+ d, Au$ ($d=d,s,b$ and $u=u,c)$
and $b^\prime \to H^+ u, Ad$ ($d=d,s,b$ and $u=u,c)$,
followed by $H^+ \to W^+ h, t \bar b$ and $A \to hZ, t \bar t$. Indeed, such decay patterns
can also lead to some un-explored collider signatures of the 4G2HDM.
We leave the discussion of the phenomenology of such
wider range of 4G2HDM scenarios to a later work.

Finally, we wish to comment on the flavor violating structure of the 4G2HDM and its
compatibility with the recently reported indications of the LFV
decay of the 125 GeV light Higgs $h \to \tau \mu$ \cite{ATLAS2,CMS2}.
Writing the LFV couplings of $h$ in a general form:
\begin{eqnarray}
{\cal L}(h f_i f_j) = {\cal S}_{ij} +  {\cal P}_{ij} \gamma_5 ~,
\end{eqnarray}
one obtains:
\begin{eqnarray}
\Gamma(h \to \bar f_i f_j + \bar f_j f_i) = \frac{m_h}{4 \pi} \left(
|{\cal S}_{ij}|^2 + |{\cal P}_{ij}|^2 \right) ~.
\end{eqnarray}

In our 4G2HDM we have for the case of the LFV decay $h \to \tau \mu$
(neglecting terms of ${\cal O}(m_\mu/m_\tau)$, see Eq.~\ref{Sff1}):
\begin{eqnarray}
|{\cal S}_{\tau \mu}| = |{\cal P}_{\tau \mu}| \sim
\frac{g}{4} \frac{m_\tau}{m_W}  f(\beta,\alpha) \xi_{\tau \mu}~,
\end{eqnarray}
where we have defined
$\Sigma^\ell_{32} = \Sigma^\ell_{23} \equiv \xi_{\tau \mu}$ (see Eq.~\ref{sigma}) and:
\begin{eqnarray}
f(\beta,\alpha) = \frac{\cos(\beta - \alpha)}{s_\beta c_\beta} ~.
\end{eqnarray}

Requiring now that $BR(h \to \tau \mu) \:\raisebox{-0.5ex}{$\stackrel{\textstyle<}{\sim}$}\: 1\%$ we find:
\begin{eqnarray}
| f(\beta,\alpha) \xi_{\tau \mu}| \sim {\cal O}(0.1)~.
\end{eqnarray}

Thus, since for the values of $\tan\beta$ and $\alpha$ that were found to be compatible with
all data considered in the previous sections, we find
$|f(\beta,\alpha)| \sim 1-5$, and specifically $f(\beta,\alpha) \sim 1$ for
$\alpha \to -\pi/2$ and $\tan\beta \sim 0.5$, as required in order
to accommodate the 750 GeV $\gamma \gamma$ resonance (see previous section),
the 4G2HDM with $|\xi_{\tau \mu}| \:\raisebox{-0.5ex}{$\stackrel{\textstyle<}{\sim}$}\: 0.1$ can address the measured
$BR(h \to \tau \mu) \:\raisebox{-0.5ex}{$\stackrel{\textstyle<}{\sim}$}\: 1\%$ if it persists.

\section{Summary \label{sec6}}

We have revisited a class of models beyond the SM, suggested by us a few years
ago in \cite{ourpaper1}, which put together an additional Higgs doublet with a
heavy chiral 4th generation quark and lepton doublet and which have several important
and attractive theoretical features.
In particular, we focused on the so-called 4G2HDM of type I (in \cite{ourpaper1}),
in which a discrete $Z_2$ symmetry couples the ``heavy" scalar
doublet only to the heavy 4th generation fermions and the
``light" one to the lighter SM fermions.

We have confronted this model with PEWD, with the measured 125 GeV light Higgs signals
and also studied its compatibility with the recent indication of a 750 GeV $\gamma \gamma$ resonance
and with the current LHC bounds on heavy scalar resonances in other relevant channels.
We found that the CP-even heavy Higgs state of the 4G2HDM with a mass $\sim 750$ GeV
can accommodate the measured $750$ GeV excess for a rather unique
choice of the parameter space: $\tan\beta \sim 0.5$, $\alpha \sim -\pi/2$ (the Higgs mixing angle)
and with heavy chiral fermion masses
$m_{t^\prime,b^\prime} \:\raisebox{-0.5ex}{$\stackrel{\textstyle<}{\sim}$}\: 400$ GeV and $m_{\nu^\prime,\tau^\prime} \:\raisebox{-0.5ex}{$\stackrel{\textstyle>}{\sim}$}\: 900$ GeV.

We have shown that the heavy chiral quarks (and leptons) of the 4G2HDM
may have FCNC decays into the light 125 GeV Higgs plus a light-quark jet, $q^\prime \to j h$,
with branching ratios of ${\cal O}(1)$, thus leading
to some un-explored signatures of $q^\prime \bar q^\prime$ production at the LHC
and, therefore, being consistent with the current direct bounds
on the masses of new heavy fermions.
Indeed, new and rich phenomenology in $q^\prime$ - heavy Higgs systems is expected,
including possible resonance production of $q^\prime q^\prime$ pairs via either
the heavy neutral or heavy charged Higgs particles of the 4G2HDM, which leads to
high jet-multiplicity signatures, with or without charged leptons, of the form
$\bar q^\prime q^\prime \to nj +  mb + \ell W$, with $n+m+\ell=6-8$
and unique kinematic features which are related to the resonating heavy scalar
and the decay pattern of the heavy quarks.
The reconstruction of the $q^\prime q^\prime$ pairs in such high jet-multiplicity signals is very challenging and
require more thought and possibly new search strategies.

We also show that the recent indication of a percent-level branching ratio
in the LFV decay of the 125 GeV Higgs $h \to \tau \mu$, if it persists, can be readily
addressed within the distinct flavor structure of the 4G2HDM.

\bigskip
\bigskip
\bigskip
\bigskip
\bigskip
\bigskip

{\bf Acknowledgments:} We thank Pier Paolo Giardino for useful conversations.
The work of AS was supported in part by the US DOE contract \#DE-SC0012704.

\pagebreak

redpajama_set_name: RedPajamaArXiv


text:
The strongest monitor that greatly affects FPSs victory or loss, or gaming mixer for children? Variable I -O data booth repo! [TGS2022]
September 18, 2022 Nelson ALeave a comment
For 4 days from September 15th to 18th, Tokyo Game Show 2022 also has a booth that handles monitors and PC parts as well as game manufacturers. Increase.
This time, we interviewed the booth of I-O Data , which will be particularly focused on companies exhibiting PC monitors. In this booth, you can test the latest series Star Ocean 6 The Divine Force scheduled to be released by Square Enix on September 22.
In recent years, FPS games have been recognized by those other than gamers and have shown great excitement. In such an FPS game, a momentary judgment is important, and the aim and the PC specifications are divided. Meanwhile, in this TGS, I-O data exhibited monitors that change the common sense of FPS.
While the normal monitor is 60Hz, the exhibited monitor LCD-GC251RXAB is 360Hz and the refresh rate has the highest level, and it has the effect of suppressing blur and reaction lag when firing with FPS, which is the effect of suppressing the lag of the reaction. It also has black insertion function. Functions such as black insertion functions and saturation adjustments can be easily changed from the remote control, and can be switched quickly until the enemy is contacted.
The angle and top and bottom of the monitor can be adjusted quite freely, and it seems that the monitor arm is almost unnecessary. In addition, the monitor has not only HDMI but also many outlets such as USB, making it feel excellent.
The monitor introduced earlier is for FPS and competition scenes, but there are monitors for general games. The monitor in the image can play games of various genres comfortably, and the refresh rate has a sufficient performance of 160Hz.
In the booth, there is a corner that reproduces the distribution environment of the Dusted player in the Prospering Streamer Group Father's Back, and the I-O Data monitor is used. Here you can know the professional distribution environment and the game environment, and if you like FPS, you definitely want to visit. A desktop PC that reproduces the PC specifications of Pastel is also on display.
We are also focusing on various peripherals, and among them, gaming mixers for children are interesting. Normally, VCs while playing a consumer game are difficult depending on the game, and unrelated players may be asked for conversations.
If you use this gaming mixer, you can play while listening to both LINE calls and game sounds. It can be said that it is a device that was born because elementary school students have a smartphone.
In this eye-oh data booth, you could see not only new monitors but also gaming mixers for children, and I felt the attitude of delivering products not only to the core layer but also to light layers and younger people. 。
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PSVR 2: Sonys brand-new virtual reality


text:
By AYLİN ÖNEY TAN aylinoneytan@yahoo.com
How food preferences of the Chinese eating bat soup made people in the U.K. or U.S. stock up on pasta is a phenomenon that can best be explained by the butterfly effect. Of course, it is already known that this entire bat soup story was fake news, but the panic buying of pasta is real.
Dried pasta, pasta asciutta or pastasciutta as the Italians call it, is a staple food in Italy, a popular commodity in most countries. A soul nourishing comfort food, it is the cheapest and most practical food one can get their hands on. Moreover, with the global rise of the Italian kitchen, it is no longer only the food of the poor, pasta is to be found in the finest tables around the world.
In Turkey, dried pasta is called makarna, after macaroni, or machheroni, the original generic Italian names for pasta. Later these words became used for only hollow tube varieties known as elbow pasta in English. Though Turkish cuisine is rich in boiled wheaten dishes such as mantı or erişte, the arrival of makaronya, as it was first named, was a true novelty in Ottoman culinary scene in the late 1700's. Though imported from Italy, it quickly became accessible by the masses. The first ever pasta production in the Ottoman times must be in 1830 at the Selimiye Barracks in Üsküdar, on the Asian side of Istanbul, where a macaroni manufacture was started for the consumption of the army and the palace, the rest making it into Istanbul markets. In the 1913 industry reports of İzmir, there were two makarna factories in city center. Needless to say, it was one of the staple provisions of the Ottoman army in the Battle of Gallipoli in 1915.
When we go back to the history of makarna as we know it, the word macaroni is recorded in Genoa city archives as early as 1279. By solid evidence, the myth that Marco Polo brought the art of pasta from China is totally a culinary legend, as he did not make it back home till 1295 from his journey from the Far East. Of course, the Chinese have been boiling innumerous varieties of noodles way before any other culture, at least from 1100 B.C, but in Italy it has its own history. This culinary myth originates from American macaroni producers as a way to popularize their products.
One of the first encounters of Americans with pasta happened at the highest level when the third president, Thomas Jefferson, ordered a pasta-making device from Napoli in 1789. Though the voyage of pasta from the Old World to the New World started at the presidential level, the image of macaroni was later associated with lower levels, especially with the influx of an almost five million Italians coming to America between 1880 and 1921. The social strata of Italian immigrants in the early nineteenth century were in pretty dim condition, so the National Association of Macaroni and Noodle Manufacturers of America (today NPA-National Pasta Association) sought for other ways to romanticize the history of pasta. It was in an ad in the Macaroni Journal that appeared in 1929, when the first Marco Polo twist appeared. The ads of the period used to be in the form of long narrative stories, so it was like a believable make-up, perhaps one of the biggest promotion success stories ever.
The story is hilariously unbelievable, it goes as such: Marco Polo was cruising his way in China Sea to exotic lands on an Italian sailing boat (the Italians must have found the way around Africa way before Vasco da Gama), one crew member going ashore spots locals made long threads of dough, reports it back to the ship, and guess what? That crew member was named Macaroni. At that point, I'd say that it should be Macarono, or whatever, if not referring to a group of Mafioso brothers in defense of elbow pasta. Nevertheless, a culinary legend was born, embarrassingly repeated by so many so-called food authorities, a fakelore still not extinguished totally.
While the popularization of pasta was happening outside Italy, there was a wave of un-popularizing pasta in its home country. Interestingly there is a belief that Mussolini tried to ban pasta. A New York Times news dated Aug. 8, 1926 writes exactly this: "The climax of Fascism has been reached. Nothing since the black shirts were first donned can compare in its way with the importance of Premier Mussolini's announcement that spaghetti must go — its place to be taken by potatoes — to help conserve wheat."
Actually, Mussolini did not ban pasta, but scorned it, but also, in a way, paradoxically encouraged the growth of durum wheat for its production. Today, in Italy pasta is a way of life. It is an identity card of Italians even beyond the national anthem or flag. As we see, all nations beyond borders, people are stocking their pantry with dried pasta. It is a proven fact that pasta unites everybody in a strange way. In Italy, it united the nation, equating rich and poor, north and south alike.
Now it is the time of equinox, when day and night is equated. Let it be the day for the world uniting over a box of pasta as their sole choice of sustenance food. This pasta mania spreading as fast as Covid-19 gives me hope, a hope that will hopefully make the world's people reach consensus on saving the planet, and I want to say just as the Italians say nowadays: "Andrá tutto bene."
People's Alliance looks to expand with conservative party
There is no breaking with Trump legacy


One of the big bonuses at Expo is the chance to see market-tested menu items prepared by the talented pizza makers who developed them. Watch these chefs put a pizza or appetizer together, hear them talk about the techniques that make their creations stand out and taste the results — all for free in the Demonstration Area on the Exhibit Hall floor.
According to a recent survey by Deloitte, 83% of respondents said that the typical fast food menu didn't offer enough healthy choices.
However, while, for the most part, pizza contains healthy ingredients, most people place it on the "banned" list if they are looking to curb calories and eat healthier.
Americans are obsessed with pizza. As our unofficial national food, there's nothing quite like a heavenly pie topped with generous heapings of cheese and sauce. But baked dough with toppings is not an exclusively American or even an Italian culinary tradition.


text:
CMOOR Group Announces Access Control Specialist Online Course
Based on strong customer demand in the industry, the CMOOR Group has released the Access Control Specialist Level One Online Course on its continuing education portal, SecurityCEU.com.
The course, which is divided into six modules, covers everything from doors, frames and electrified locking devices to the latest in smartcards and biometrics. Students who take the course will receive both CEU credits as well as certification from SecurityCEU.com online academy.
"The course will demystify access control," said Connie Moorhead, president of The CMOOR Group. "And there is nothing else like it available in the industry for security sales reps, technicians, installers, IT professionals and systems integrators."
The Access Control Overview module is the foundation on which the rest of the Access Control Specialist Level One certification is built. Module 1 provides a thorough overview of access control, beginning with doors and hardware, locks and lock history, door position in monitoring and egress control and ending with the components of an electronic access control system.
Module 2 covers credentials and readers including magnetic stripe, Wiegand swipe, 125 kHz proximity, contact and contactless smartcards and combination cards. Module 3 deals with binary math and the various card data formats, and will teach students how to choose the right format every time. Module 4 presents smartcard technology and details contact and contactless smartcards, applications for EAC systems, smartcard security, mutual authentication, multiple applications on the card and global platform.
Module 5 includes a high-level overview of the most popular biometric technologies such as fingerprint, hand geometry, iris recognition and facial recognition. The difference between passive and active biometric systems is also covered. Module 6, the final module, starts with a short review of the components that make up an access control system, and then looks at various options ranging from single door stand-alone devices to widely distributed systems using IP connections over LAN/WAN networks. Wiring standards are explained as well as the idea of POE (Power Over Ethernet) and Integration of CCTV with access control.
"We already have online courses in structured wiring, NICET Fire, CCTV, IP networking and now we have introduced a very thorough access control course, which integrates with our other courses. We've got the industry covered," Moorhead said.
Each of the six modules is available for $40, while the complete Level 1 Training Bundle will be sold for $200, a $40 savings. There are also deep volume discounts for 10 or more students.


text:
How To Make Red Stretch Marks White
The Truth About Treating Stretch Marks Red Vs. White
Pulsed dye laser therapy is a painless blast of light used on new, red stretch marks. The light's energy calms blood vessels under your skin that could cause the marks.... The appearance of stretch marks can be attributed to constant contraction and then relaxation of the delicate tissue which results in the loss of flexibility. Moisturizing skin will help you get rid of those stretch marks faster use type of lotions that contain shea butter and cocoa butter and drink more water!
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From puberty to pregnancy, stretch marks can occur at any time of life for a variety of reasons. Ways to remove these pesky marks include topical creams and tummy tucks. LEARN MORE ›... On a basic level, stretch marks appear to be similar to superficial scarring. Typically they start off with a reddish cast, and then settle down into permanent lines that are either paler or
The white of the egg is rich in protein and this is useful in dealing with stretch marks. Collect the whites from two eggs, whip gently and apply as a thick layer onto the marks. how to make navy blue icing Stretch marks are purple-red streaky scars that appear in overstretched skin. Many adolescents and about half of all pregnant women will develop stretch marks. Over time, stretch marks lose their red or purple colour and become white or silvery streaks.
Stretch marks are considered one of the most common beauty concerns which can develop in both men and women as a result of sudden changes in body size. They appear as pink, red or purple marks on the skin which will fade to a thin silvery white or gray color overtime. how to make dairy free alfredo sauce Stretch marks are considered one of the most common beauty concerns which can develop in both men and women as a result of sudden changes in body size. They appear as pink, red or purple marks on the skin which will fade to a thin silvery white or gray color overtime.
HOW TO GET RID OF STRETCH MARKS!! YouTube
Laser Stretch Marks Does It Work? Expert Answers
Both red stretch marks and white stretch marks can be noticed on the stomach and the belly as well. Pregnancy lines is a term used in describing stretch marks on the stomach among women. The pregnancy lines form on the belly after and during the pregnancy.
Stretch marks, the lines that develop on the abdomen, as well as on other areas of the body, are a common skin concern in pregnancy. While they pose no risk at all to mother or baby, the discomfort created if they lead to itching, not to mention the cosmetic effects of their appearance, can cause pregnant women much distress.
31/12/2018 · Stretch marks typically start out as red streaks, but usually fade to pink or white over time. Although it is unlikely that they will ever go away without surgery, for most people they become much less noticeable after a few months to a year. The texture of the scar usually remains, however.
20/09/2018 · "Active" stretch marks tend to be red or purple, fading toward silvery white over time, Is there a faster way to make your stretch marks disappear? Chris M. Matsko, MD Family Medicine Physician Dr. Matsko is a retired Physician in Pennsylvania. He received his M.D. from the Temple University School of Medicine in 2007. Chris M. Matsko, MD. Family Medicine Physician. Expert …
• Red stretch marks (striae rubra) — These form because of the overstretching of the dermal layer of the skin. People with red stretch marks will notice that the blood vessels in the layer below are visible.
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text:
The 2015 Ivy League Softball Championship Series was held at Dartmouth Softball Park in Hanover, New Hampshire, the home field of  on May 2, 2015.  The series matched the regular season champions of each of the league's two divisions.  The winner of the series claimed the Ivy League's automatic berth in the 2015 NCAA Division I softball tournament. All games in the series would be broadcast on the Ivy League Digital Network.

 claimed the Rolfe Division title while  won the Gehrig Division, making the third consecutive season Dartmouth and Penn would face off for the right to advance to the NCAA Tournament. In the end Dartmouth would walk away with their second consecutive Ivy League title.

Results
Game One

Game Two

References

Ivy League Championship
Tournament, 2015


text:
Northeast: Chara surpasses the 1000-game mark
By John-Eric Iannicello
Photo: Boston Bruins captain Zdeno Chara played in his 1000th game on Saturday night vs. the Los Angeles Kings (courtesy of
Ric Tapia/Icon SMI)
Saturday night's contest against the Los Angeles Kings was a historic event for the Boston Bruins' captain, Zdeno Chara. Chara played his 1000th career NHL game, a career that started 13 seasons ago with the New York Islanders on November 19th, 1997 against the Detroit Red Wings.
"On the way here I thought about how it all started and it's a lot of games," Chara told ESPN.com. "I caught myself thinking, 'Where did all the time and games go?' It's unbelievable because when you're playing it seems like it's a long season and long year but when you reach this kind of number you're like, 'Oh my God, it went so fast,' and that's what it tells you that you have to enjoy it, you have to do your best and have fun. It's going to go by fast and before you know it you have to hang your skates so I was thinking about that and how lucky I am."
Selected 56th overall by the New York Islanders in 1996, Chara played three seasons with the Islanders before being dealt in 2001. The deal that sent Chara to the Ottawa Senators would end up being (arguably) the franchise's greatest trade in their history. The Senators acquired Chara, along with Bill Muckalt and the second-overall pick in the 2001 NHL Entry Draft which ended up becoming franchise center Jason Spezza. The Senators ended up shipping enigmatic forward Alexei Yashin to the Islanders in the deal.
Chara's career really started to soar with the Senators. As a 24-year-old, Chara's offensive potential started to flourish, scoring 10 goals in his first season as a Senator in 2001. The following year, Chara finished second in team defensive scoring to Wade Redden with nine goals and 30 assists, while also leading the team with a +29 rating.
The blossoming defenseman would go on to play two more seasons with the Senators before a management decision to sign Wade Redden left the then 29-year-old open to unrestricted free agency. He would go on to sign a five-year, $37.5 million dollar contract with divisional rival Boston on July 1st, 2006.
Since joining the Bruins, Chara's been to the NHL All-Star Game four times, has won the James Norris Memorial Trophy for Defenseman of the Year and Mark Messier Leader of the Year Award, and was named the NHL Plus/Minus Leader last season. He's also captained the Bruins to the Stanley Cup in 2010-11.
Chara has arguably been the most dominant NHL defender in recent memory. His menacing shot from the point (clocking in at 108.8 mph) strikes fear to everyone on the ice, and his physical attributes are second to none in the league.
"He's gotten better every year and at the same time, he's just kind of blossomed into a real great captain and every year you see him continuing to grow no matter what his age is," Bruins coach Claude Julien told Bruins.com." He wants to continue to get better, he wants to continue to learn, he wants to be better on the ice, better off the ice."
Chara and the Bruins came away with a victory on the night of his 1000th game, beating the Los Angeles Kings 4-2 on Saturday night. The Slovakian defender has 136 goals and 315 assists in his career and is also a +142.
Northeast Division Notes
Boston Bruins: Boston wrapped up their Western road trip on Sunday night with a 3-2 win against the Anaheim Ducks. On Saturday, Tim Thomas turned aside 40 shots for the 4-2 win over the Los Angeles Kings. The Bruins signed draftees Justin Florek, 21, and Zach Trotman, 21, to entry-level deals this weekend. The club also announced the signing of free agent NCAA defenseman Torey Krug to an entry-level contract on Sunday. Krug was formerly a member of Michigan State.
Buffalo Sabres: The surging Sabres came away with key back-to-back victories this weekend over the New York Rangers and Minnesota Wild. Ryan Miller played in both contests and only allowed two goals. Cody Hodgson continued his recent offensive streak, contributing a goal and assist on Saturday. The club has collected 16 out of a possible 20 points in their past 10 games.
Montreal Canadiens: Erik Cole scored three goals in the first six minutes of Friday's contest vs. the Senators. His third goal in the game was also his 30th of the season. Cole has scored 30 goals once in his career, and it's also his career high for goals in a season. Defenseman Frederic St-Denis was recalled from Hamilton (AHL). The Canadiens ended up splitting the weekend with a 5-1win over the Senators and a 4-1 loss the following night against the Philadelphia Flyers. Hall of Famer Jean Beliveau was released from hospital on Saturday after suffering a stroke in February.
Ottawa Senators: Craig Anderson returned to the crease on Friday night after missing the last four weeks with an injury hand. Anderson was pulled after allowing two goals on four shots. He was returned to the net at the start of the second period. Erik Condra and Jason Spezza hit career markers in games played this weekend. Spezza played in his 600th game, while Condra reached the 100-game mark.
Toronto Maple Leafs: James Reimer turned aside 43 shots in the Maple Leafs 4-3 shootout win on Friday in New Jersey. Nazem Kadri and Ryan Hamilton were both returned to the Marlies on Sunday. Kadri recorded a goal and Hamilton added an assist in Friday night's shootout victory. Hamilton's assist was his first career NHL point. Both forwards were on emergency recall to replace injured forwards Clarke MacArthur and Matt Frattin.


text:
SunflowRenderer::~SunflowRenderer() {

	delete sc.image;
	delete sc.camera;
	delete sc.gi;

	for (int i = 0; i < sc.shaders.size(); i++) {
		delete sc.shaders[i];
	}

	sc.shaders.clear();

	for (int i = 0; i < sc.lights.size(); i++) {
		delete sc.lights[i];
	}

	sc.lights.clear();

	for (int i = 0; i < sc.objects.size(); i++) {
		delete sc.objects[i];
	}

	sc.objects.clear();
}

string SunflowRenderer::bid() {

	int n = 0;

	if (sc.image) {
		n++;
	}
	if (sc.camera) {
		n++;
	}
	if (sc.gi) {
		n++;
	}
	n += sc.lights.size();
	n += sc.shaders.size();
	n += sc.objects.size();

	stringstream ss;
	// 'b' means 'block'
	ss << "b" << n;
	return ss.str();
}

void SunflowRenderer::call() {

	stringstream options;

	if (option.output != "") {
		options << " -o " << getBinDir() << "/" << option.output << " ";
	}

	if (option.nogui) {
		options << " -nogui ";
	}

	if (option.ipr) {
		options << " -ipr ";
	}

	stringstream ss;
	ss << "cd " << SF_LIB_PATH << ";";
	ss << "./sunflow " << options.str() << formatPath;

	string command = ss.str();
	if (system(command.c_str()) != -1) {
		cout << "[INFO] execute " << ss.str() << endl;
	} else {
		cout << "[ERROR] sunflow render command error has occured." << endl;
		cout << ss.str() << endl;
		exit(0);
	}
}

void SunflowRenderer::clear() {

	currShader = 0;

	for (int i = 0; i < sc.shaders.size(); i++) {
		delete sc.shaders[i];
	}

	sc.shaders.clear();

	for (int i = 0; i < sc.lights.size(); i++) {
		delete sc.lights[i];
	}

	sc.lights.clear();

	for (int i = 0; i < sc.objects.size(); i++) {
		delete sc.objects[i];
	}

	sc.objects.clear();
}

void SunflowRenderer::flush(string name) {

	sc.image->flush(bufferStream);
	sc.camera->flush(bufferStream);
	sc.gi->flush(bufferStream);

	for (int i = 0; i < sc.lights.size(); i++) {
		sc.lights[i]->flush(bufferStream);
	}

	for (int i = 0; i < sc.shaders.size(); i++) {
		sc.shaders[i]->flush(bufferStream);
	}

	BoxGenericMeshBlock box;
	box.flush(bufferStream);

	for (int i = 0; i < sc.objects.size(); i++) {
		sc.objects[i]->flush(bufferStream);
	}

#ifdef false
	bufferStream.dump();
#endif

	bufferStream.save(name);
}

void SunflowRenderer::render() {

	// save sc
	string name = SF_SC;
	flush(name);

	// set sc path
	formatPath = bufferStream.getPath();

	// start rendering
	call();
}

void SunflowRenderer::render(string format) {

	formatPath = getBinDir() + "/" + format;

	// start rendering
	call();
}

void SunflowRenderer::setImageResolution(int width, int height) {
	sc.image->resolution = vec2f(width, height);
}

void SunflowRenderer::setFilter(string filter) {
	sc.image->filter = filter;
}

void SunflowRenderer::smooth(const int min, const int max) {
	sc.image->aaMin = min;
	sc.image->aaMax = max;
}

void SunflowRenderer::setupScreenPerspective(const vec3f eye, const vec3f target, const vec3f up, const float fov, const float aspect) {

	if (sc.camera) {
		PinholeCameraBlock* camera = dynamic_cast<PinholeCameraBlock*>(sc.camera);
		camera->eye = eye;
		camera->target = target;
		camera->up = up;
		camera->fov = fov;
		camera->aspect = aspect;
	} else {
		sc.camera = new PinholeCameraBlock(eye, target, up, fov, aspect);
	}
}

void SunflowRenderer::setAmboccBright(const Color bright) {

	AmbientOcclusionBlock* ambocc = dynamic_cast<AmbientOcclusionBlock*>(sc.gi);

	if (ambocc) {
		ambocc->bright = bright;
	}
}

void SunflowRenderer::setAmboccDark(const Color dark) {

	AmbientOcclusionBlock* ambocc = dynamic_cast<AmbientOcclusionBlock*>(sc.gi);

	if (ambocc) {
		ambocc->dark = dark;
	}
}

void SunflowRenderer::setAmbocc(const Color bright, const Color dark, const int samples, const float maxdist, const string colorSpace) {

	AmbientOcclusionBlock* ambocc = dynamic_cast<AmbientOcclusionBlock*>(sc.gi);

	if (ambocc) {
		ambocc->bright = bright;
		ambocc->dark = dark;
		ambocc->samples = samples;
		ambocc->maxdist = maxdist;
		ambocc->colorSpace = colorSpace;
	} else {
		sc.gi = new AmbientOcclusionBlock(bright, dark, samples, maxdist, colorSpace);
	}
}

void SunflowRenderer::setPointLight(const vec3f _position, const Color _color, const float _power, const string _colorSpace) {
	sc.lights.push_back(new PointLightBlock(_position, _color, _power, _colorSpace));
}

void SunflowRenderer::setColor(const float r, const float g, const float b, const float a) {

	// search shader
	for (int i = 0; i < sc.shaders.size(); i++) {

		Color c = sc.shaders[i]->getColor();

		if (c.r == r && c.g == g && c.b == b && c.a == a) {
			// set current shader
			currShader = dynamic_cast<ShaderBlock*>(sc.shaders[i]);
			return;
		}
	}

	DiffuseShader* shader = new DiffuseShader(bid(), Color(r, g, b, a), SF_COLORSPACE_SRGB_NONLINEAR);
	sc.shaders.push_back(shader);

	// set current shader
	currShader = dynamic_cast<ShaderBlock*>(shader);
}

void SunflowRenderer::sphere() {

	matrix4x4 m;
	glPushMatrix();
	glScalef(.5f, .5f, .5f);
	glGetFloatv(GL_MODELVIEW_MATRIX, m.getPtr());
	glPopMatrix();

	SphereBlock* sphere = new SphereBlock(bid());
	sphere->m = m;

	if (currShader) {
		sphere->shader = currShader->getName();
	}

	sc.objects.push_back(sphere);
}

void SunflowRenderer::box() {

	matrix4x4 m;
	glGetFloatv(GL_MODELVIEW_MATRIX, m.getPtr());

	InstanceBlock* box = new InstanceBlock(bid(), "\"Box\"");
	box->m = m;

	if (currShader) {
		box->shader = currShader->getName();
	}

	sc.objects.push_back(box);
}

void SunflowRenderer::quads(vector<vec3f> vertices) {

	matrix4x4 m;
	glGetFloatv(GL_MODELVIEW_MATRIX, m.getPtr());

	QuadsBlock* quads = new QuadsBlock(bid());
	quads->vertices = vertices;
	quads->m = m;

	if (currShader) {
		quads->shader = currShader->getName();
	}

	sc.objects.push_back(quads);
}

void SunflowRenderer::floor() {

	matrix4x4 m;
	glGetFloatv(GL_MODELVIEW_MATRIX, m.getPtr());

	// name value have to be unique if using instance
	PlaneBlock* plane = new PlaneBlock(bid());
	plane->m = m;
	plane->p = vec3f(0, 0, 0);
	plane->n = vec3f(0, 1, 0);

	if (currShader) {
		plane->shader = currShader->getName();
	}

	sc.objects.push_back(plane);
}

redpajama_set_name: RedPajamaGithub


text:
Beacon grad Radwan sues UConn over soccer scholarship
HARTFORD, Conn. - A former UConn soccer player from Wappingers Falls who lost her scholarship after giving the middle finger to a television camera said she is suing the school, calling her punishment excessive.
Noriana Radwan, who now plays for Hofstra, held a news conference Monday in Newburgh. Her lawyer said the lawsuit would be filed later in the day in U.S. District Court in Connecticut.
Radwan graduated from Beacon High School in 2014 and is a former Poughkeepsie Journal all-star.
LOOK BACK: UConn soccer player, a Beacon grad, suspended
She made the obscene gesture to an ESPNU camera while celebrating with teammates after the Huskies beat the University of South Florida 3-2 on penalty kicks in the 2014 American Athletic Conference championship game.
Coach Len Tsantiris initially suspended Radwan from the 2014 NCAA Tournament and issued a statement apologizing to the conference, USF and those who watched the game on television.
In her federal lawsuit, a draft of which was given to The Associated Press, Radwan alleges that, after the publicity died down, she was stripped of her scholarship midway through the school year without due process for what the coach described as "serious misconduct."
Radwan said she wrote a letter of apology to UConn officials after the incident, which the school never acknowledged. She also apologized Monday.
"I did not intend to offend anyone. I was making a celebratory statement that was seriously misinterpreted and misjudged," she Radwan said in a prepared statement. "I loved UConn, but I lost faith in it as an institution when it allowed my scholarship to be illegally taken away so abruptly and crassly in the middle of the school year, violating all trust I had."
She is seeking monetary damages.
"What she really wants is to make sure something like this does not happen to any other young woman," said Greg Tarone, her lawyer said.
Tarone also said that, while Radwan's offense was regrettable, it hardly rises to the level of "serious misconduct," and the punishment was much harsher than what male athletes at the school have received for more serious offenses.
He said a UConn football player, offensive lineman Brian Cespedes, was not even suspended from his team after he was being arrested Dec. 10 on misdemeanor assault charges stemming from a September incident that was not public at the time.
"It's clear from the information I've gathered that there have been many other incidents of much more serious misconduct and nobody lost a scholarship over it," Tarone said.
The school has not seen the lawsuit and cannot comment on it because of federal privacy laws, said UConn spokeswoman Stephanie Reitz.
Radwan, a midfielder, played in nine games for the Huskies as a freshman. She did not have a goal.
She transferred to Hofstra, where she is on a partial athletic scholarship. She started 17 games this past season, scoring six goals and adding an assist.


text:
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Genetics: Books For Kids
Looking for a list of the best children's books about genetics?
Curated by Bookroo: The Children's Book Experts
As you can see, this list of kids books about genetics is a work in progress! We're currently exploring the best books available, and we'd love your input. If you have a title you'd suggest including on our list of kids books about genetics, please share it with us!
We'll be featuring a variety of titles on our list, from well known classics to popular bestsellers to lesser known titles that deserve a bigger audience. We're also including books for a range of ages, from board books for babies and toddlers, to picture books for preschool and kindergarten age kids, to chapter books for early elementary age kids.
We'd love to hear any book suggestions you have—you can comment below or email us at [email protected].
Have a Nice DNA
Written by Fran Balkwill and Mic Rolph
Recommend Ages: 3-9
Enjoy Your Cells is a new series of children's books from the acclaimed creative partnership of scientist/author Fran Balkwill and illustrator Mic Rolph. Once again, they use their unique brand of simple but scientifically accurate commentary and exuberantly colorful graphics to take young readers on an entertaining exploration of the amazing, hidden world of cells, proteins, and DNA. It's over ten years since Fran and Mic invented a new way of getting science across to children. Think what extraordinary advances have been made in biology in that timeand how often those discoveries made headlines. Stem cells, cloning, embryo transfer, emerging infections, vaccine developmentELhere in these books are the basic facts behind the public debates. With these books, children will learn to enjoy their cells and current affairs at the same time. And they're getting information that has been written and reviewed by working scientists, so it's completely correct and up-to-date. Readers aged 7 and up will appreciate the stories' lively language and with help, even younger children will enjoy and learn from the jokes and illustrationsno expert required! This series is a must for all elementary school students and those who care about educating them to be well-informed in a world of increasingly complex health-related and environmental issues.
Used $4.85
Prices as of Jan 19
Gene Machines
Enjoy Your Cells is a new series of children's books from the acclaimed creative partnership of scientist/author Fran Balkwill and illustrator Mic Rolph. Once again, they use their unique brand of simple but scientifically accurate commentary and exuberantly colorful graphics to take young readers on an entertaining exploration of the amazing, hidden world of cells, proteins, and DNA. It's over ten years since Fran and Mic invented a new way of getting science across to children. Think what extraordinary advances have been made in biology in that time–and how often those discoveries made headlines. Stem cells, cloning, embryo transfer, emerging infections, vaccine development–here in these books are the basic facts behind the public debates. With these books, children will learn to enjoy their cells and current affairs at the same time. And they're getting information that has been written and reviewed by working scientists, so it's completely correct and up-to-date. Readers aged 7 and up will appreciate the stories' lively language and with help, even younger children will enjoy and learn from the jokes and illustrationsno expert required! This series is a must for all elementary school students and those who care about educating them to be well-informed in a world of increasingly complex health-related and environmental issues.
Used $13.11
I Miss My Grandpa
Written & illustrated by Jin Xiaojing
For fans of Ed Young and Peter Sis, this breathtaking picture book, from LBYR's first Emerging Artist Award Winner, Jin Xiaojing, is the perfect read for anyone who has lost a loved one.
A young girl has never met her grandpa. He passed away before she was born, but she misses him every day. She often wonders…what did he look like? Grandma says: His face was shaped like the moon, his mouth was good at telling stories, and his hair was as curly as a bird's nest. With the help of her grandma and the rest of her loving family, will this young girl be able to imagine her grandpa's face in her mind–and feel the love that he shared with others?
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text:
The attack that shook Twitter is now hitting several companies
Last month, three young men were arrested in the United Kingdom and the United States, accused of one of the biggest scams ever suffered by Twitter. They managed to control the account of famous personalities like Joe Biden, Jeff Bezos and Elon Musk through a well known technique.
Long before this security breach became public, dozens of victims suffered the same blow, and in recent weeks a wave of crime has taken off on a grand scale.
In July, Twitter announced that hackers had used a technique called "phone snoop", literally translated "phone sniper", which allowed them to view 130 accounts, including CEOs, politicians and celebrities. Hackers managed to take control of 45 of these accounts, using them to send tweets promoting a pyramid scheme. Bitcoin .
Twitter wrote on your blog about this intrusion, reporting that hackers contacted Twitter employees using false identities to gain access to credentials that gave them access to an internal tool of the company itself that would allow them to reset passwords and authentication settings for multiple accounts.
But Twitter hasn't been the only recent "telephone fishing" target, just in the last month, since the Twitter hack went public, dozens of companies, including banks and web hosting companies, have been targeted by the same attack.
As in the Twitter attack, employees of these targets received phone calls from hackers posing as tech staff to trick them into giving their passwords to internal tools. Attackers then sold that access to others.
These attacks use the so-called social engineering, it exploits security holes in human processes that allow the invasion without even needing as much technical knowledge. Attacks of this size and organization have never been seen before being carried out by independent groups, normally an attack of this magnitude is carried out by specialized groups and even governments, leaving investigators intrigued to discover that everything was orchestrated by a few teenagers around the world.
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