text:
The Russo Brothers' SLUGFEST Series Will Chronicle the DC Vs. Marvel Rivalry
by Eric Diaz
This year, the Russo Brothers took a large chunk of Marvel Comics' heroes and propelled them into becoming the biggest movie stars of all time with Avengers: Endgame. And although they may be done telling fictional stories with those characters for now, that doesn't mean they are done with Marvel all together. According to a report coming from Variety, producers Anthony and Joe Russo will soon be bringing a new show to the upcoming Quibi streaming service documenting the long rivalry between comic book publishers Marvel and DC.
The series, called Slugfest, will be based on Reed Tucker's book Slugfest: Inside the Epic, 50-Year Battle between Marvel and DC. Slugfest will be directed by Don Argott and Sheena M. Joyce, directors of the award-winning documentaries Believer and Framing John DeLorean. This is the latest high profile project coming from the soon-to-launch streaming service Quibi, which already has projects from names such as Steven Spielberg, Sam Raimi, and Guillermo del Toro.
DC Comics / Marvel Comics
Slugfest will include some of the lesser known stories from both Marvel and DC's long histories, and will contain interviews with several creators from both powerhouse publishers.
Among the confirmed moments being highlighted is the 1976 Superman vs. The Amazing Spider-Man comic, the first time the rivals agreed to share their two biggest characters for a single story. The success of that comic led to other temporary cease-fires between the two publishers, producing noteworthy comics like Batman vs. The Hulk, Uncanny X-Men and The New Teen Titans, and the biggest one of all, JLA/Avengers.
The rivalry between Marvel and DC has actually always been beneficial to both publishers. In the '60s when Stan Lee and Jack Kirby changed comics with the beginnings of the Marvel Universe, DC was still the premiere publisher. But during that era, most DC titles were fairly simplistic and aimed at a very young audience. Marvel pushed the boundaries of comic book storytelling, which then forced DC to push the envelope themselves in order to stay relevant. The rivalry kept both publishers on their toes, and making great comics.
Another aspect of the long standing DC vs. Marvel Comics war that will no doubt be touched on is the battle over certain creators. Jack Kirby invented most of the Marvel icons in the '60s, and then left for DC to invent the New Gods mythology. Years later, writer/artist John Byrne helped elevate the X-Men and Fantastic Four comics into top sellers during the '80s, only for DC to steal him away and have him perform that same magic trick with the Superman books. The most recent example of this is perhaps Jim Lee, a superstar artist who made X-Men the biggest selling comic of all time. Today, he's DC Comics' co-publisher.
It will be interesting to see if the docuseries will extend to the DC vs Marvel rivalry that's happening now in live-action media. What was once confined to the niche audience of comics has now spilled over to the mainstream, with movie going audiences picking their sides in the war. Given their involvement in the Marvel Studios films, it will be fascinating to see how the Russo Brothers approach that particular aspect of the long standing DC/Marvel cold war.
Slugfest doesn't have a release date yet. However, Quibi will be launching in April 2020.
Featured Image: Marvel Comics / DC Comics
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Filippo Grippaldi has been active in the field of old masters for the past 30 years as an advisor and restorer. He opened his first gallery in the Principality of Monaco in 2004. The Grippaldi Gallery essentially offers paintings by European masters from the 14th to the 20th century
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ARMAN, Armand Pierre Fernandez dit, (Nice 1925 - 2005 New York), "Colère", 1962 Courtesy de Gianenzo Sperone, Galerie Grippaldi
EXHIBITIONARMAN, LES ANNEES 60 April 24th - June 4th
We could call it the golden decade. The twelve works presented here were created between 1961 and 1970, ten years during which Arman contributed actively to one of the most remarkable artistic adventures of the century, the New Realism (nouveau réalisme), and developed processes that made his creations into his own personal adventure.
In 1960, Arman exhibited with Jacques Villeglé, Jean Tinguely and Raymond Hains at the Galleria Apollinaire in Milan. Pierre Restany, the theorist of the group, writes: "We are moving towards the new realism of pure sensitivity. Man, if he manages to reintegrate into reality, identifies it with his own transcendence, which still is emotion, feeling, and, ultimately, poetry". A few months later, the same artists, along with Yves Klein, François Dufrene, Martial Raysse, and Daniel Spoerri, signed, in Paris, the manifesto of the New Realists. The impulse was given. For Arman, it stopped only with his death.
At the time, like other members of the group, Arman could not make a living as an artist; he was sustaining himself with small jobs. But it is the production of artworks which keeps him busy. Inventions and discoveries are linked together. Abandoning the painting itself, the artist launches his Cachets, made of imprints of tampons repeated at will. Then come the Allures, color impressions of some object trace on a support. A turn was taken. Moving from the object used as a tool (Allure) to the object considered as a work of art, Arman gives birth to accumulations which constitute, in the words of Bernard Lamarche-Vadel, the backbone of the artist's approach. Exhibited in New York in 1961, these accumulations influenced a young Andy Warhol, a year before he exhibited himself his famous Campbell's Soup. It is also worth mentioning the Colères (destroyed objects) and the Poubelles , typical productions of the artist.
With the accumulations Arman, encouraged by the experiences of his predecessors (dadaists, and ready made, artworks by Marcel Duchamp), holds the emergence of a new perspective on the urban and industrial society, its production and waste.
The déchets (waste) therefore constitute the Bacille (1961), an accumulation of used films reels and Sans titre of 1963 (rusted screws). Modern industrial production is a primary objective for Arman for example in the accumulated electric coils (Sans titre 1961), the aluminum disks (Clinibare EDF, 1962) the valves of oxygen tanks (Oxygénation, 1964), moreover he plays with the colors of the fuses electrical (Sans titre, 1964) and with electrical components (Cloud Burst, 1968).
The car being the industrial object par excellence, in 1967 Arman concluded an agreement with Renault, that provided the artist with spare parts and raw materials for the famous Renault Accumulations that two years later was exhibited in Berlin (Kunshalle), Amsterdam (Stedelijk Museum), and Paris (Museum of Decorative Arts).
Among these works we can find our accumulation of electric wires, maliciously entitled Spaghetti sauce Renault.
Even if the Accumulations are mass-produced objects, Arman's Colères concern "noble" objects, and more often on musical instruments. Sans titre (1962) shows a violently broken guitar by the artist. The gesture is more surgical in the Colère de violons (1970), the instruments have been carefully cut before being presented. With the Accumulation de téléphones (1969) and Violons éclatés, apparently between colère and accumulation, the destructive violence is followed by a highly studied staging.
Effectively, recognition arrived in these fruitful years, in Europe as in the United States, where Arman spent part of the year. In 1964, the artist organized his two first solo exhibitions at the Minneapolis Walker Art Center and the Stedelijk Museum. During the same year, he received the Second Prize at the Tokyo Biennial and, in 1966, the Marzotto Grand Prix. The consecration came with in 1968 the participation in two among the most significant artistic events: the Venice Biennal and the Dokumenta of Kassel. The artworks presented there witness the emergence and affirmation of an artist who is now considered one of the greatest of his century.
ARMAN, Armand Pierre Fernandez dit, (Nice 1925 - 2005 New York)

redpajama_set_name: RedPajamaCommonCrawl


text:
\section{Introduction}
Theoretical description of water adsorption on micro- and mesoporous materials is a challenge problem for modern physical chemists and chemical engineers. Its great importance is due to numerous industrial applications and fundamental significance of describing water in a nanoconfinement. The examples of technological applications, where the description of water adsorption is highly relevant, are: characterizing of micro- and mesoporous materials at ambient conditions (i.e. determination of pore size distribution, surface area, accessible volume) \cite{Russo2007,Groenquist2019,Georgi2017,kolesnikov2018effects,kolesnikov2017pore,landers2013density}, modelling of water purification from toxic compounds (e.g., ions of heavy metals \cite{peng2017review}), description of mechanical stability of construction porous materials (concrete, wood, paper, etc.) during capillary condensation/evaporation cycles\cite{hamouda2002influence,jakovljevic2017influence,trong2018sorption,setzer1974surface} , {\sl etc}. All these examples have one common feature - the influence of inhomogeneity on the process.

Obtaining a correct description of inhomogeneous water requires a reliable theoretical model based on the first principles of statistical mechanics. Such a theoretical model must account for the electrostatic interactions (including short-range specific interactions, attributed to electron charge transfer) between water molecules and must be based on the nonlocal functional theory to describe correctly the liquid-vapour interface and temperature behavior of the surface tension. Despite the fact that up to now several theoretical models have been formulated \cite{Yang1994, Ding1987, Lischner2010, Jaqaman2004, Fu2005, Hughes2013, Krebs2014, Chuev2006, Trejos2019,trejos2018theoretical}, none of them satisfy the requirements formulated above.

In paper \cite{Yang1994} the authors formulated a density functional theory (DFT) taking account of the molecular structure of water within the TIP4P model \cite{Jorgensen1983} for describing the water liquid-vapour interface. The authors took into consideration the universal intermolecular interactions by the Lennard-Jones pair potential, whereas the electrostatic interactions between sites -- through the Coulomb potentials. To take into account for the electrostatic interactions in the total free energy functional, the authors used the mean-field approximation, expanding the anisotropic potential into the multipole series, truncated by the fifth order. They applied the local density approximation with the Weeks Chandler Andersen (WCA) procedure to the dispersion interactions \cite{andersen1971relationship}. Though the authors obtained rather satisfactory agreement with the experimental liquid-vapour coexistence curve (binodal), the values of the surface tension at all the temperatures were  highly overestimated. Such a discrepancy can be explained in two ways. Firstly, the authors used the local DFT and, thus, did not take into account the nonlocal packing effects which should be important for the water molecules, situated at the interface. Secondly, the authors did not consider the many-body electrostatic correlations of the water molecules which must be significant in condensed liquid phase. Indeed, while for a vapour phase the electrostatic correlations manifest themselves through the effective Keesom pairwise interactions, for the liquid condensed phase it is necessary to take into account the higher electrostatic correlations \cite{Budkov2018, Budkov2019}.  Nevertheless, from the result of the manuscript\cite{nezbeda2005towards}
one can conclude that the main electrostatic contribution comes from the short-range part of the Coulombic potential. The author shows that short-range attractive and repulsive interactions play the crucial role in the structure properties of polar and associating pure fluids. Later in the work \cite{rodgers2008interplay}
the authors pointed out that not accounting for the long-range electrostatic interactions leads to errors in the system with non-uniform geometries, however mostly errors arise in electrostatic properties.

It is also necessary to mention the phenomenological density functional theories of water which do not take into account the electrostatic interactions explicitly \cite{Ding1987,Lischner2010,Jaqaman2004,Fu2005,Krebs2014,Hughes2013}. In paper \cite{Ding1987} the authors formulated a molecular DFT of water, which allowed authors to predict with good accuracy the  temperature of freezing at atmospheric pressure. To perform the numerical calculations, the authors used the experimental pair correlation functions oxygen-oxygen, oxygen-hydrogen, and hydrogen-hydrogen. Thus, despite the success of formulated molecular DFT, its application to different molecular systems requires the external experimental data regarding the site-site correlation functions (from X-ray scattering or full-atomistic computer simulations). In paper \cite{Lischner2010} the authors used a similar molecular phenomenological DFT approach to describe the liquid-vapour interface of water at a temperature of $298~K$. Despite the fact that the authors obtained a good fitting for experimental values of densities of the coexisting phases and surface tension, it remained unclear how this approach could describe these quantities at the other state parameters. Moreover, the formulated theory deals with the polynomial approximation for the excess free energy, whose phenomenological coefficients are not related to any statistical theory. In paper \cite{Jaqaman2004} the authors developed a phenomenological DFT which operates with the position-orientation number density of structured fluids. Despite the fact that this theory is based on the bulk equation of state, describing the anomalous behavior of water below $4^{0}~C$ and taking explicit account of the hydrogen bonding between the water molecules, whereas the free energy functional accounts for the nonlocality through the gradient term, the surface tension obtained is twice its experimental value. As the authors mentioned \cite{Jaqaman2004}, this discrepancy is most probably due to the simplicity of the gradient correction used. In paper \cite{Fu2005} a self-consistent DFT, taking explicit account of hydrogen bonding through the Statistical Associating Fluid Theory (SAFT) \cite{Wertheim1984}, is applied to investigating the phase behavior and surface tensions of water and aliphatic alcohols. The authors showed that for the bulk phases, their theory is reduced to an equation of state that provides an accurate description of saturation pressures as well as vapor-liquid phase diagrams. Near the critical region, the long-range fluctuations were taken into account using a renormalization group theory. It is worth mentioning the similar SAFT-based density functional approach \cite{Krebs2014,Hughes2013}, where the authors not only described the saturation pressure and surface tension, but also analyzed the effective interactions between the hydrophobic hard rods, immersed in liquid water. In the manuscript\cite{gloor2007prediction}, the authors used the SAFT-VR density functional theory in order to describe the vapor-liquid interface of associating and non-associating molecules, including water. The functional treats short-range repulsion, chain and association contributions in the local density approximation. A good description of both binodal and surface tension was achieved by including interfacial data in the optimization scheme \cite{gloor2007prediction}. In the work \cite{sundararaman2014efficient}, the authors developed classical density-functional theory of rigid-molecular fluid and applied it to calculations of thermodynamic and structural properties of water. The used functional contains the hard-spherical contribution (White Bear mark II), contribution of the attractive Van der Waals interactions (on the weighted-density approximation level), and electrostatic contribution, described within the mean-field approximation. The using hard-sphere diameter as a fitting parameter allowed authors to describe surface tension with good accuracy.

Despite the fact that in the mentioned papers the authors obtained a very good fitting for the saturation pressure and liquid-vapour surface tension, these are only a few theories accounting explicitly the electrostatic interactions between water molecules. The existing SAFT-based density functional theories can be considered as good tools for chemical engineering applications, but cannot answer the physically reasonable question: How big the contribution of the electrostatic interactions between water molecules to the surface tension of the liquid-vapour interface? Moreover, in principle, the SAFT-based theories in their present form cannot elucidate the role of the electrostatic correlations in the capillary phenomena taking place with confined water.

One of the simplest water models is the SPC/E  - a 3-site model. Each site carries a point-like charge and additionally, the Lennard-Jones interaction potential between oxygen atoms is applied. Despite the fact that SPC/E model does not take into account hydrogen bonding explicitly, it can reproduce some thermodynamic and structural properties with sufficient accuracy \cite{Alejandre1995, vega2007surface}. Inspiring the fact that such a simple model allowed the authors to describe equilibrium water in MD simulations, we will formulate a nonlocal simple DFT approach for the description of inhomogeneous liquid water. Describing water molecules as spherically symmetric dipolar particles, having two oppositely charged sites and taking into account the many-body electrostatic correlations, universal inter molecular interactions, and short-range specific interactions, related to electron charge transfer, we will describe with good accuracy the binodal and the surface tension at ambient conditions. In the framework of the formulated theory, we will elucidate the role of different inter molecular interactions in the chemical potential of water at the liquid-vapour interface.

\section{Theory of bulk water}
Let us formulate a simple statistical theory of liquid (vapour) water in the bulk phase. We describe each water molecule as two sites with charges $\pm q$, separated by distance $l$, so that the dipole moment is $p=ql=1.85~D$.  We assume that sites with charges $-q<0$ interact with each other through the Coulomb potential, the Lennard-Jones (LJ) potential, and the attractive square-well short-range potential (see the description below). The sites with a charge $+q>0$ interact with all types of sites through the Coulomb potential only. We would like to note that the LJ potential describes the excluded volume and dispersion interactions, while the square-well potential takes into account at the primitive level the short-range specific interactions between water molecules. In other words, in this study we do not take explicit account of the association between water molecules, resulting in the formation of a hydrogen bond network. Instead, we replace the asymmetric chemical interactions by the effective spherically symmetric short-range square-well potential. Such a simplification is quite acceptable, because in this study we do not consider the fine effects, related to the network of the hydrogen bonds (see, for instance, \cite{Jorgensen1998,Holten2012}). As we will show below, such a primitive description of the effect of chemical interactions will allow us to describe the liquid-vapour coexistence curve and surface tension of water at the normal conditions that are the goal of the present study. Note that explicit account of the association effect was made in the general context in papers \cite{SEGURA1997,Yu2002,Haghmoradi2016,Erukhimovich2002,Trejos2019,trejos2018theoretical}. We also neglect the effect of static electronic polarizability of water molecules, as it is much less than the orientation polarizability, related to the permanent dipole moment at the normal temperature. Due to the fact that our model is the first statistical theory of liquid water taking into account dipole correlations of molecules at the many-body level within the random phase approximation, we have neglected for simplicity the orientation nonlinear effects, such as formation of chain-like clusters in accordance with $"$head-to-tail$"$ mechanism taking place usually in magnetic and ferroelectric fluids \cite{klapp2005dipolar,budkov2019nonlocal}. As we will show below, such an assumption allows us to describe successfully the phase coexistence curve and surface tension of liquid-vapour interface of water at the ambient conditions.

Bearing in mind all the above written model assumptions, we can write the density of Helmholtz free energy of water as follows:
\begin{equation}
f(\rho,T) = f_{id}(\rho,T)+f_{ex}(\rho,T),
\end{equation}
where
\begin{equation}
f_{id}(\rho,T)=\rho k_{B}T\left(\ln(\rho \lambda^3)-1\right)
\end{equation}
is the free energy of the ideal gas.
The excess free energy can be written in the following form
\begin{equation}
f_{ex}(\rho,T)=f_{sr}(\rho,T) + f_{el}(\rho,T),
\end{equation}
where
\begin{equation}
\label{fLJ}
f_{sr}(\rho,T)=\rho k_B T \left(-\ln(1 - \eta) + \frac{3\eta}{1 - \eta} + \frac{3 \eta^2}{2(1 - \eta)^2}\right)+\frac{1}{2}B \rho^2,
\end{equation}
is the contribution of the short-range interactions, including the excluded volume interactions, dispersion interactions, and short-range specific interactions; $B$ is the parameter of attractive interactions accumulating the contributions from WCA attraction tail
\[
V_{WCA}(|\mathbf{r}|)=
\left\{
\begin{tabular}{ccc}
  $-\epsilon$ & ~if~ & $r < 2^{1/6}\sigma$ \\
  $4\epsilon\left[\left(\frac{\sigma}{r}\right)^{12} - \left(\frac{\sigma}{r}\right)^{6}\right]$ & ~if~ & $2^{1/6}\sigma < r < r_c$ \\
  $0$ & ~if~ & $r > r_c$ \\
  \end{tabular}
  \right\}
 \]
and
\begin{equation}
V_{spc}(|\mathbf{r}|)=-\epsilon_{sw}\Theta(\sigma_{sw}/2-|\mathbf{r}|),
\end{equation}
where $r_{c}$ is the cutoff of LJ pairwise potential of interactions; $\Theta(r)$ is the Heviside step-function; $\sigma$ and $\epsilon$ are, respectively, the size and energy parameters of LJ potential; $\epsilon_{sw}$ and $\sigma_{sw}$ are, respectively, the energy and size parameters of the square-well potential. The latter describes the contribution of short-range specific interactions \cite{goodwin2017mean,budkov2018theory} which in our case is related to the electron charge transfer of the water molecules. We assume for our calculations that $r_{c}=5\sigma$. Such an assumption allows us to make our DFT calculations (see the next section) less time-consuming \cite{neimark1998pore}. The first term in (\ref{fLJ}) describes the contribution of the excluded volume interactions of the hard spheres within the Percus-Yewick approximation; $\eta= \pi d_{BH}^3\rho/6 $ is the packing fraction of hard spheres with the effective Barker-Henderson diameter, determined by the following Pade approximation \cite{Verlet1972a}
\begin{equation}
d_{BH} = \sigma\frac{1.068 \epsilon/k_B T + 0.3837}{\epsilon/k_B T + 0.4293}.
\end{equation}
 The second term in (\ref{fLJ}) describes the total contribution of the attractive interactions, thus $B$ can be defined as:
 \begin{equation}
     B =\int d\mathbf{r} \biggl(V_{WCA}(|\mathbf{r}|) + V_{spc}(|\mathbf{r}|) \biggr) = -\frac{32\sqrt{2}}{9}\pi\epsilon\sigma^3 + \frac{16}{3}\pi\epsilon\sigma^3\left[ \left(\frac{\sigma}{r_c}\right)^3 - \frac{1}{3}\left(\frac{\sigma}{r_c}\right)^9\right] -\frac{\pi\epsilon_{sw}\sigma_{sw}^3}{6}.
 \end{equation}

The contribution of the electrostatic interactions, which in our case are reduced to the short-range dipole-dipole interactions, can be described by the free energy of the dipolar hard spheres (see Appendix 1):
\begin{equation}
f_{el} = -\frac{k_B T}{l^3} \left(1-\frac{3}{4}\alpha\right)\sigma(y),
\end{equation}
where $l$ is the dipole length and $y = \rho p^2/3 \epsilon_0 k_B T$, $p$ is the dipole moment. The auxiliary function
\begin{equation}
\sigma(y) = \frac{\sqrt{6}}{4\pi}\left[2(1+y)^{3/2}-2-3y\right]
\end{equation}
is also introduced; the compressibility factor $\alpha$ of the hard spheres (see Appendix 1) in Percus-Yevick approximation has the following form
\begin{equation}
\alpha=\frac{\eta(4-\eta)(2+\eta^2)}{(1+2\eta)^2}.
\end{equation}
 Before that, we talk only about the thermodynamic properties, however, it is interesting to study also the structural ones. Here, we compare calculated structure factor and pair correlation function of the homogeneous water at 298 K with presented literature experimental data and DFT calculations. In general, there are two methods to calculate pair correlation function within DFT - test particle method and method base on the Ornstein-Zernike (OZ) equation. Recently \cite{archer2017standard}, it was shown that the first one gives more accurate results and especially enforce the correct behavior at small distances. However, we unable to use it due to the lack of explicit known form of the effective electrostatic pair potential, thus we will use OZ-based method (see  Appendix IV). The Fourier transform of structure factor in the homogeneous limit can be calculated by the standard expression \cite{hansen1990theory}:
\begin{equation}
S(k) = \frac{1}{1 - \rho c^{(2)}(k)},
\end{equation}
where $k=|\bold{k}|$; the pair correlation function can be expressed through structure factor as:
\begin{equation}
g(r) = 1 + \frac{1}{2 \pi^2 r \rho } \int \limits_0^{\infty} dk k\sin(kr)(S(k) - 1). \label{g_eq}
\end{equation}

\begin{figure}[h!]
\center{\includegraphics[width=1\linewidth]{FigS.pdf}}
\caption{Comparison between calculated structure factor at ambient temperature and average intermolecular structure factor obtained from x-ray measurements\cite{badyal2000electron}. }
\label{struct}
\end{figure}

\begin{figure}[h!]
\center{\includegraphics[width=1\linewidth]{FigG.pdf}}
\caption{Comparison between pair correlation function calculated within the present approach, spherically averaged site-site correlation function oxygen-oxygen for scaler-EOS water functional\cite{sundararaman2014efficient} and x-ray measurements at ambient conditions.\cite{hura2000high}  }
\label{gOO}
\end{figure}

Figures \ref{struct} and \ref{gOO} represent the comparison between structure factor calculated within this model, molecular density functional theory \cite{sundararaman2014efficient}, and X-Ray scattering experiments \cite{hura2000high,badyal2000electron}. We obtain only partial qualitative agreement between our model and X-Ray obtained structure factor. Our results does not demonstrate the split of first pick \cite{bopp1996static} and the next picks, on bigger $k$, are shifted to the left. The first pick approximately corresponds to the average position of the first experimental ones and the amplitudes of picks are in agreement with experimental data. By means of Eq.(\ref{g_eq}) we calculated the pair correlation function. The Fig. \ref{gOO} represents X-Ray obtained \cite{hura2000high} and calculated within cDFT \cite{sundararaman2014efficient} $g_{OO}$,  and $g(r)\Theta(r - d_{HS})$ calculated in the present study. We plotted only part of the whole pair correlation function (cutted approximately on the distance of effective hard-sphere diameter), due to the numerical artifacts on the low distances. The pair correlation function does not go to zero in the core region. Such behavior was already previously reported in the literature \cite{archer2017standard} and can be attributed to the accuracy of the used method. Nevertheless, the obtained pair correlation function is in a good agreement with the results of molecular density functional theory except the position of the first maximum. The latter is shifted to the higher values by approximately 0.3 $\si{\angstrom}$. However, we would like to note that both theories fail to reproduce the real structure of water and demonstrates a significant shift of the second and third picks.

\section{Nonlocal density functional theory of inhomogeneous water}
Based on the bulk theory which was formulated in the previous section, let us formulate a density functional theory of inhomogeneous water. We start from the grand thermodynamic potential of inhomogeneous water in external potential field with the potential energy $V_{ext}(\bold{r})$, which can be written in the following form
\begin{equation}
\Omega[\rho(\mathbf{r})] = F_{id}[\rho(\mathbf{r})] + F_{ex}[\rho(\mathbf{r})]+\int_V d\mathbf{r} \rho(\mathbf{r}) V_{ext}(\mathbf{r}) - \mu\int_V d\mathbf{r} \rho(\mathbf{r}), \label{GTP}
\end{equation}
where $V$ is system volume, $F_{id}[\rho(\mathbf{r})]$ is the free energy of the ideal gas, $F_{ex}[\rho(\mathbf{r})]$ is the excess free energy of water, $\mu$ is the chemical potential and $\rho(\bold{r})$ is the single-particle density. Note that within this consideration $\rho(\bold{r})$ is the average density of the centers of mass of the water molecules. Thus, we construct the effective nonlocal DFT in terms of the simple fluid theory \cite{hansen1990theory} for water that is a molecular liquid in its nature. Such a simplification can be considered as an example of coarse-graining. The ideal gas free energy is
\begin{equation}
F_{id}[\rho(\mathbf{r})] = k_B T \int_V d\mathbf{r} \rho(\mathbf{r})[\ln(\lambda^3\rho(\mathbf{r})) - 1]
\end{equation}
and the excess free energy, in turn, consists of several parts:
\begin{equation}
F_{ex}[\rho(\mathbf{r})] = F_{sr}[\rho(\mathbf{r})] + F_{el}[\rho(\mathbf{r})],
\end{equation}
where
\begin{equation}
F_{sr}[\rho(\mathbf{r})] = F_{fmt}[\rho(\mathbf{r})] + F_{att}[\rho(\mathbf{r})]
\end{equation}
with the Helmholtz free energy $F_{fmt}[\rho(\mathbf{r})] $ of hard spheres with the effective BH diameter $d_{BH}$ within the fundamental measure theory (FMT) \cite{rosenfeld1989free}, namely
\begin{equation}
F_{fmt}[\rho(\mathbf{r})] = \int_V d\mathbf{r} \Phi(\{n\}),
\end{equation}
where the free energy density is
\begin{equation}
\Phi(\{n\}) =k_{B}T\left(-n_0\ln(1 - n_3) + \frac{n_1 n_2 - \mathbf{n}^{(v)}_1 \mathbf{n}^{(v)}_2}{1 - n_3} + \frac{n_2^3 - 3 n_2 \mathbf{n}^{(v)}_2 \mathbf{n}^{(v)}_2}{24 \pi (1 - n_3)^2}\right),
\end{equation}
which depends on six weighted densities:
\begin{equation}
n_{\alpha}(\mathbf{r}) = \int_V d\mathbf{r}^{\prime}\omega_{\alpha}(\mathbf{r} - \mathbf{r}^{\prime}) \rho(\mathbf{r}^{\prime}),
\end{equation}
where $\omega_{\alpha}(|\mathbf{r} - \mathbf{r}^{\prime}|)$ are the weight functions. Four of them are scalar values: $\omega_{2}(\mathbf{r}_{12}) = \delta(d_{BH}/2 - |\mathbf{r}_{12}|)$, $\omega_{3}(\mathbf{r}_{12}) = \Theta(d_{BH}/2 - |\mathbf{r}_{12}|)$, $\omega_{1}(\mathbf{r}_{12}) = \omega_{2}(\mathbf{r}_{12}) / (2\pi d_{BH})$, $\omega_{0}(\mathbf{r}_{12}) = \omega_{2}(\mathbf{r}_{12}) / (\pi d_{BH}^2)$,  and two are vector values: $\mathbf{\omega}^{(V)}_{2}(\mathbf{r}_{12}) = \mathbf{r}_{12}/r_{12}\delta(d_{BH}/2 - |\mathbf{r}_{12}|)$ and $\mathbf{\omega}^{(v)}_{1}(\mathbf{r}_{12}) = \mathbf{\omega}^{(v)}_{2}(\mathbf{r}_{12})/(2\pi d_{BH})$. The functional $F_{att}[\rho(\mathbf{r})]$ is the contribution from the given above attractive potentials $V_{WCA}(\bold{r})$ and $V_{spc}(\bold{r})$:
\begin{equation}
F_{att}[\rho(\mathbf{r})] = \frac{1}{2}\int\int_V d\mathbf{r}_1d\mathbf{r}_2\rho(\mathbf{r}_1)\rho(\mathbf{r}_2)\biggl[V_{WCA}(|\mathbf{r}_1 - \mathbf{r}_2|) + V_{spc}(|\mathbf{r}_1 - \mathbf{r}_2|)\biggr].
\end{equation}

Note that we do not know the real electrostatic free energy functional of dipolar hard spheres. On the other hand, due to the fact that thermodynamic properties of strongly inhomogeneous confined polar fluids must be very different from those are in the bulk phase, we cannot use the local density approximation for the electrostatic free energy functional. Nevertheless, since we know the approximate expression for the electrostatic free energy of the dipolar hard spheres system for the bulk phase, we can construct the phenomenological weighted density functional based on it, using the Curtin-Ashcroft-Tarazona approach \cite{curtin1985weighted,tarazona1985free,hansen1990theory}. We would like to note, that using of the weighted density functional approach can be justified by the fact that electrostatic interactions between water molecules in liquid phase manifest themselves as the effective short-range dipole-dipole interactions \footnote{This is related to the fact that the bulk electrostatic free energy of dipolar hard spheres system can be expanded into the power series on density (virial expansion), in contrast to the ionic systems, for which the electrostatic contribution to the total free energy is not an analytic function of density. As is well known, non-analytical behavior of electrostatic free energy of the ionic systems is determined by the long-range electrostatic interactions and translation entropy of ions \cite{landau2013course}. However, if the ionic groups form the electrically neutral clusters, as in dipolar \cite{Budkov2018,Budkov2019} or quadrupolar \cite{budkov2019statistical} fluids, the effective interactions between particles become short-range and, thereby, analyticity of the electrostatic free energy recovers.}. Thus, following the idea of the weighted density functional theory \cite{curtin1985weighted,tarazona1985free}, we treat the electrostatic free energy functional as follows:
\begin{equation}
F_{el}[\rho(\mathbf{r})] = \int_V d\bold{r}\rho(\mathbf{r}) \phi_{el}(\bar{\rho}(\mathbf{r})),
\end{equation}
where $\phi_{el}(\bar{\rho}(\mathbf{r})) = f_{el}(\bar{\rho})/\bar{\rho}$ is the free energy per fluid particle, depending on smoothed density, which, in turn, is determined in the following way:
\begin{equation}
\bar{\rho}(\mathbf{r}) = \int_V d\mathbf{r^{\prime}} \rho(\mathbf{r^{\prime}}) \omega_{el}(|\mathbf{r^{\prime}} - \mathbf{r}|),
\end{equation}
where $\omega_{el}(|\mathbf{r}|) = 3/(4\pi R_w^3)\Theta(R_w -|\mathbf{r}|)$ is the phenomenological weighted function with the phenomenological scale parameter $R_w$ determined the range of smoothing.

The equilibrium density profile is obtained from the minimization of the grand thermodynamic potential (\ref{GTP}), i.e. from the Euler-Lagrange equation
\begin{equation}
\frac{\delta\Omega[\rho(\mathbf{r})]}{\delta \rho(\mathbf{r})}=0
\end{equation}
or
\begin{equation}
\rho(\mathbf{r}) = \rho \exp \left[\beta(\mu_{ex} - V_{ext}(\mathbf{r})) + c^{(1)}(\bold{r})\right],
\end{equation}
where
\begin{equation}
\nonumber
c^{(1)}(\bold{r})=-\frac{\delta \left(\beta F_{ex}[\rho]\right)}{\delta\rho(\bold{r})}=c^{(1)}_{fmt}(\bold{r}) + c^{(1)}_{WCA}(\bold{r}) +c^{(1)}_{spc}(\bold{r}) + c^{(1)}_{el}(\bold{r})
\end{equation}
is the one-particle direct correlation function; $\beta=(k_{B}T)^{-1}$ is the inverse thermal energy; $\mu_{ex}=\mu_{ex}(\rho,T)$ is the bulk excess chemical potential, given in Appendix II. The contributions to the one-particle direct correlation function can be written as
\begin{equation}
c^{(1)}_{el}(\mathbf{r}) =-\frac{\delta \left(\beta F_{el}[\rho]\right)}{\delta\rho(\bold{r})}= -\beta\phi_{el}(\bar{\rho}(\mathbf{r})) - \beta\int_V d\mathbf{r^{\prime}} \rho(\mathbf{r^{\prime}}) \left[ \frac{\mu_{el}(\bar{\rho}(\mathbf{r^{\prime}}))}{\bar{\rho}(\mathbf{r^{\prime}})} - \frac{\phi_{el}(\bar{\rho}(\mathbf{r^{\prime}}))}{\bar{\rho}(\mathbf{r^{\prime}})} \right] \omega_{el}(|\mathbf{r} - \mathbf{r^{\prime}}|),
\end{equation}
\begin{equation}
c^{(1)}_{WCA}(\mathbf{r}) = -\frac{\delta \left(\beta F_{WCA}[\rho]\right)}{\delta\rho(\bold{r})}=-\beta \int_V d\mathbf{r^{\prime}}\rho(\mathbf{r^{\prime}})V_{WCA}(|\mathbf{r} - \mathbf{r^{\prime}}|),
\end{equation}
\begin{equation}
c^{(1)}_{spc}(\mathbf{r}) =-\frac{\delta \left(\beta F_{spc}[\rho]\right)}{\delta\rho(\bold{r})}= -\beta \int_V d\mathbf{r^{\prime}}\rho(\mathbf{r^{\prime}})V_{spc}(|\mathbf{r} - \mathbf{r^{\prime}}|),
\end{equation}
\begin{equation}
c^{(1)}_{fmt}(\mathbf{r}) =-\frac{\delta \left(\beta F_{fmt}[\rho]\right)}{\delta\rho(\bold{r})}= -\beta\sum\limits_{\alpha}\int_V d\mathbf{r^{\prime}}\frac{\partial \Phi(\{n\})}{\partial n_{\alpha}}\omega_{\alpha}(\mathbf{r^{\prime}} - \mathbf{r})
\end{equation}
Note that the formulated DFT for the bulk phase, where $V_{ext}(\bold{r})=0$ and, thus, $\rho(\bold{r})=\rho=const$, transforms into the bulk theory discussed in the previous section.

\section{Numerical results and discussions}
Now we will consider the application of the model to the description of water liquid-vapour interface. We used the theory formulated above to fit the experimental values of coexisting densities and surface tension at the ambient temperature $T=298~K$. In order to calculate the densities of coexisting phases, we used the following system of equations, consisting of mechanical and chemical equilibrium conditions, i.e.
\begin{equation}
P(\rho_v,T) = P(\rho_l,T)~~ and~~ \mu(\rho_v,T) = \mu(\rho_l,T),
\end{equation}
where $\rho_v$ and $\rho_l$ are, respectively, the densities of the coexisting vapor and liquid phases. To calculate the equilibrium density profile, we used slit geometry with the length $H = 30\sigma - 60\sigma$ and discretization step along $z$ axis $\approx 0.02\sigma$. The surface tension was calculated by the following relation
\begin{equation}
\gamma=\Omega[\rho(z)]/A + PH,
\end{equation}
where $\Omega[\rho(z)]/A$ is the part of the grand thermodynamic potential per unit area $A$ corresponding to the liquid-vapour and $P$ is the pressure in the bulk liquid and vapour phases. The expressions for the pressure and chemical potential are given in Appendix II. The detailed description of DFT main equations in slit geometry is presented in Appendix III. Note that the obtained pressure at $T=298~K$ is deviated from the experimental value ($\approx 3141.7~kPa$) less than 1 $\%$. It is worth noting that the latent heat of vaporization at $298~K$ is $\approx 40.89~kJ/mol$, with experimental value $44~kJ/mol$. Thus, fitting the densities $\rho_v$ and $\rho_l$ and the surface tension $\gamma$ yields the following set of microscopic parameters:
\begin{center}
Table I: The obtained set of parameters for water.
\end{center}
\begin{center}
\begin{tabular}{ ||c c c c c c|| }
 $\sigma$ (\r{A}) & $\epsilon$ (kcal/mol) & $\sigma_{sw}$ (\r{A}) & $\epsilon_{sw}$(kcal/mol) & $l$ (\r{A}) & $R_w$ (\r{A})\\
 3.01 & 0.447 & 6.02 & 1.68 & 2.8 & 3.01
\end{tabular}
\end{center}
Using these model microscopic parameters, we calculated the binodal and surface tension at other temperatures. Fig. \ref{binodal} shows the comparison between the binodal, calculated within our DFT, molecular simulations of Alejandre et al. \cite{Alejandre1995} and Vega et al\cite{vega2007surface}, and the experimental one \cite{lemmon1998thermophysical}.
\begin{figure}[h!]
\center{\includegraphics[width=1\linewidth]{Fig1.pdf}}
\caption{Liquid-vapour coexistence curves, obtained from the experiment (squares), molecular simulations (points), and present theoretical model (solid line).}
\label{binodal}
\end{figure}
\begin{figure}[h!]
\center{\includegraphics[width=1\linewidth]{Fig2.pdf}}
\caption{Dependences of surface tension on temperature, obtained from our density functional theory, the classical density functional theories presented in the literature and experiment. Worth noting that surface tension calculated within another two works \cite{sundararaman2014efficient,Yu2002} are in almost perfect agreement with exprimental data in the wide range of temperatures and will be barely visible on the present figure.}
\label{surf_tens}
\end{figure}

\begin{figure}[h!]
\center{\includegraphics[width=1\linewidth]{Fig2a.pdf}}
\caption{Dependences of surface tension on temperature, obtained from our density functional theory, molecular simulations, and experiment.}
\label{surf_tens_1}
\end{figure}
As one can see, the theoretical binodal is in very good agreement with both the MD simulation and the experiment at the ambient state parameters. However, our theory slightly underestimates the critical density and overestimates the critical temperature. However, this disagreement between the theoretical and experimental critical points is not very important for applications discussed in the Introduction. Fig. \ref{surf_tens} demonstrates a comparison between the dependences $\gamma~vs~T$, obtained from our DFT  and SAFT-based DFT \cite{Hughes2013,Krebs2014, gloor2007prediction}. The surface tension values calculated within our DFT agree very well with the experimental values at the ambient temperatures and deviate significantly only at sufficiently high temperatures that are close to the critical one. The latter is related to the fact that our theory cannot describe correctly the liquid-vapour equilibrium in the critical point vicinity. As is seen from fig. \ref{surf_tens}, the same picture is observed for the SAFT-based DFT \cite{Krebs2014,Hughes2013, vega2007surface}. We do not show the surface tension calculated in the works \cite{sundararaman2014efficient,Yu2002}. The results obtained in them are almost in a perfect agreement with experimental data.  Fig. \ref{surf_tens_1} demonstrates the comparison between our DFT, molecular simulations \cite{Alejandre1995, vega2007surface}, and experimental measurements \cite{lemmon1998thermophysical}. The surface tension obtained by different authors within one water model (SPC/E) are  different, which could be due to differences in the simulation procedures\cite{vinvs2016molecular}. The results of the present DFT is in quantitative agreement with TIP4P72005 water model. Further, we compared the density profile at the liquid-vapour interface calculated within our DFT the MD simulation with profiles available in the literature \cite{taylor1996molecular} and {\sl ab initio} Car-Parinello simulations \cite{kuhne2010new}. As Figures \ref{dens_prof1} and \ref{dens_prof2} show, our theory reproduces the simulation density profiles quite well. Note that DFT density profiles were shifted horizontally in order to match the regions of the steep descent of the simulated ones.

Despite the good consistent of the calculated surface tensions with experimental and simulation data, the density profiles are significantly steeper than simulation ones. That can be clearly identified by the comparison of the decaying length in the following equation \cite{hansen1990theory}:
\begin{equation}
\rho(z) = \frac{1}{2}(\rho_v + \rho_l) - \frac{1}{2}(\rho_l - \rho_v) \tanh\left(\frac{z-z_0}{d}\right),
\end{equation}
where $\rho_v$ and $\rho_l$ are vapor and liquid densities, $z_0$ is a position of the Gibbs dividing surface and $d$ is the decay length. The same form was used in the work \cite{vega2007surface}, where the authors reported the value of "10-90" thicknesses ($t = 2.1972 d$) for density profiles calculated in the SPC/E, TIP4P and TIP4P/2005 water models at $300~K$. They are 3.39 $\si{\angstrom}$, 3.67 $\si{\angstrom}$ and 3.22 $\si{\angstrom}$, respectively. The value obtained in the present model is approximately $2$ times lower $\approx 1.76$ $\si{\angstrom}$.
Also, density profiles demonstrate slightly more pronounced oscillation behavior than those are obtained from molecular simulations.

\begin{figure}[h!]
\center{\includegraphics[width=1\linewidth]{Fig3.pdf}}
\caption{Density profile at the liquid-vapour interface of water at temperature $T=298~K$, calculated from our DFT (solid line) and from MD simulations of Taylor et al (symbols).}
\label{dens_prof1}
\end{figure}

\begin{figure}[h!]
\center{\includegraphics[width=1\linewidth]{Fig4.pdf}}
\caption{Density profile at the liquid-vapour interface of water at temperature $T=300~K$, calculated within our DFT (solid line) and taken from MD simulations of Kuhne et al (symbols).}
\label{dens_prof2}
\end{figure}

It is instructive to estimate the contributions of different intermolecular interactions to the excess chemical potential of liquid water predicted by our statistical model. Fig. \ref{chem_pot} shows these contributions as the functions of temperature, calculated along the liquid-phase branch $\rho_{l}=\rho_{l}(T)$ of the binodal. As is seen, the contribution of the universal intermolecular interactions ($\mu_{LJ}$) and electrostatic contribution ($\mu_{el}$) almost compensate for each other at all the temperatures, so that the total excess chemical potential in the liquid state region within our model is determined by the contribution of short-range specific interactions ($\mu_{spc}$). This prediction, in principle, could be verified by {\sl ab initio} Car-Parinello computer simulations \cite{kuhne2010new}.
\begin{figure}[h!]
\center{\includegraphics[width=1\linewidth]{Fig5.pdf}}
\caption{Contributions of different intermolecular interactions to excess chemical potential of water as functions of temperature, calculated along the liquid-phase branch of the binodal.}
\label{chem_pot}
\end{figure}
\section{Concluding remarks and prospects}
We have formulated a nonlocal density functional theory of inhomogeneous liquid water. We considered a water molecule as a couple of oppositely charged sites. The negatively charged sites interact with each other via the Lennard-Jones potential, square-well potential, and Coulomb potential, whereas the positively charged sites interact with all types of sites via the Coulomb potential only. Taking into account the nonlocal packing effects in the framework of the fundamental measure theory, dispersion and specific interactions in the mean-field approximation, and electrostatic interactions at the many-body level through the random phase approximation we have described the liquid-vapour interface. Namely, we have shown that our model without explicit account of the association of water molecules and with explicit account of the many-body electrostatic interactions at the many-body level is able to describe the liquid-vapour coexistence curve and the surface tension at ambient state parameters with good accuracy.

In conclusion, we would like to discuss the prospects of the formulated density functional theory. At first, this theory could be used as a theoretical background for describing the capillary phenomena, such as wetting/dewetting and capillary condensation/evaporation occurring at the solid surfaces of micro- and mesoporous materials. However, we cannot guarantee that application of this theory to the description of confined water will not change the values of the microscopic parameters of water molecules. However, we believe that the obtained microscopic parameters will be quite close to those obtained in the present study. The density functional theory of confined water will allow us to characterise micro- and mesoporous materials using the experimental adsorption isotherms of water vapour. Secondly, the formulated theory can be used for describing thermodynamic properties of other bulk and confined polar fluids, such as dimethylformamide, aliphatic alcohols, etc. However, these issues are the subject of forthcoming publications.

\section*{Conflicts of interest}
There are no conflicts to declare.

\begin{acknowledgements}
The model development was supported by the RFBR according to research project No 18-31-20015. The project was partially supported by the RFBR according to research project No 18-29-06008. The authors thank Mikhail Kiselev for fruitful discussions and valuable comments.
\end{acknowledgements}

\section{Appendix I: Derivation of Helmholtz free energy of a system of dipolar hard spheres}
In this appendix we will briefly consider the fluctuation theory of complex fluids, whose electrically neutral molecules can be modelled as a set of clusters of spatially correlated charged centers with charges $q_{\alpha}$. A simplest example of such a fluid is a polar fluid, which we will consider in detail. More specifically, we will derive within the random phase approximation (RPA) an analytical expression for the Helmholtz free energy of the dipolar hard spheres system in the bulk.  We start from fluid partition function, which can be written as the following functional integral over the fluctuations of the local number densities $\rho_{\alpha}(\bold{r})$ of the charged centers as follows
\begin{equation}
Z=\mathcal{N}\int \prod\limits_{\alpha}^{}\mathcal{D}\rho_{\alpha}\exp\left[-\beta F_{0}[\{\rho_{\alpha}\}]-\beta U_{cl}[\{\rho_{\alpha}\}]\right],
\end{equation}
where $\beta=(k_{B}T)^{-1}$ is the inverse thermal energy, $F_{0}[\{\rho_{\alpha}\}]$ is the free energy functional of the reference system without Coulomb interactions between the particles; $\mathcal{N}$ is the normalization constant which will be specified below;
\begin{equation}
U_{cl}[\{\rho_{\alpha}\}]=\frac{1}{8\pi\varepsilon_{0}}\int d\bold{r}\int d\bold{r}^{\prime}\frac{\rho_{c}(\bold{r})\rho_{c}(\bold{r}^{\prime})}{|\bold{r}-\bold{r}^{\prime}|}
\end{equation}
is the energy of Coulomb interactions between the charged centers, $\rho_{c}(\bold{r})=\sum_{\alpha}q_{\alpha}\rho_{\alpha}(\bold{r})$ is the local charge density; $\varepsilon_{0}$ is the vacuum permittivity.

Further, we expand the free energy of the reference system into the functional power series near the average densities $\bar{\rho}_{\alpha}=\rho$ of the charged centers
\begin{equation}
F_{0}[\{\rho_{\alpha}\}]\approx F_{0}[\{\bar{\rho}_{\alpha}\}]+\frac{k_{B}T}{2}\int d\bold{r}\int d\bold{r}^{\prime}
\sum\limits_{\alpha,\gamma}G_{\alpha\gamma}^{-1}(\bold{r}-\bold{r}^{\prime})\delta\rho_{\alpha}(\bold{r})\delta\rho_{\gamma}(\bold{r}^{\prime}),
\end{equation}
where $\delta\rho_{\alpha}(\bold{r})=\rho_{\alpha}(\bold{r})-\bar{\rho}_{\alpha}(\bold{r})$ is the fluctuation of the local charge densities;
\begin{equation}
G^{-1}_{\alpha\gamma}(\bold{r}-\bold{r}^{\prime})=\frac{\delta^2}{\delta\rho_{\alpha}(\bold{r})\delta\rho_{\gamma}(\bold{r}^{\prime})}\left(\frac{F_{0}}{k_{B}T}\right)\biggr\rvert_{\rho=\bar{\rho}}
\end{equation}
is the inverse structure operator of the reference system for which we adopt the following approximation
\begin{equation}
G_{\alpha\gamma}^{-1}(\bold{r}-\bold{r}^{\prime})=W_{\alpha\gamma}^{-1}(\bold{r}-\bold{r}^{\prime})-c_{\alpha\gamma}(\bold{r}-\bold{r}^{\prime}),
\end{equation}
where $c_{\alpha\gamma}(\bold{r}-\bold{r}^{\prime})$ is the matrix of direct correlation functions of the sites that are not bonded to each other and
\begin{equation}
W_{\alpha\gamma}(\bold{r}-\bold{r}^{\prime})=\rho\delta_{\alpha\gamma}\delta(\bold{r}-\bold{r}^{\prime})+\rho(1-\delta_{\alpha\gamma})g_{\alpha\gamma}(\bold{r}-\bold{r}^{\prime})
\end{equation}
is the matrix of the structure factors of molecules; $g_{\alpha\gamma}(\bold{r}-\bold{r}^{\prime})$ is the probability distribution function of the distance between the $\alpha^{th}$ and $\gamma^{th}$ sites. Thus, we have the following relation
\begin{equation}
Z\approx\exp\left[-\beta F_{0}[\{\bar{\rho}_{\alpha}\}]\right]\mathcal{N}\int \prod\limits_{\alpha}^{}\mathcal{D}\rho_{\alpha} \exp\left[-\frac{1}{2}\int d\bold{r}\int d\bold{r}^{\prime}
\sum\limits_{\alpha,\gamma}S_{\alpha\gamma}^{-1}(\bold{r}-\bold{r}^{\prime})\delta\rho_{\alpha}(\bold{r})\delta\rho_{\gamma}(\bold{r}^{\prime})\right],
\end{equation}
where
\begin{equation}
S_{\alpha\gamma}^{-1}(\bold{r}-\bold{r}^{\prime})=G_{\alpha\gamma}^{-1}(\bold{r}-\bold{r}^{\prime})+\frac{q_{\alpha}q_{\gamma}}{4\pi\varepsilon_0 k_{B}T|\bold{r}-\bold{r}^{\prime}|}
\end{equation}
is the inverse structure operator in the random phase approximation. Further, choosing the normalization constant $\mathcal{N}$ from the condition that at $q_{\alpha}=0$ the electrostatic contribution to the free energy is equal to zero and calculating the Gaussian functional integral, we arrive at
\begin{equation}
F=F_{0}+F_{el},
\end{equation}
where
\begin{equation}
\label{Fcorr3}
F_{el}=\frac{Vk_{B}T}{2}\int\frac{d\bold{k}}{(2\pi)^3}\left(\ln\left(1+\frac{\varkappa^2(\bold{k})}{k^2}\right)-\frac{\varkappa^2(\bold{k})}{k^2}\right)
\end{equation}
is the electrostatic free energy and
\begin{equation}
\varkappa^2(\bold{k})=\frac{1}{\varepsilon_0 k_{B}T}\sum\limits_{{\alpha\gamma}}q_{\alpha}q_{\gamma}G_{\alpha\gamma}(\bold{k})
\end{equation}
is the screening function. Note that we have subtracted from the final expression the electrostatic self-energy of the molecules
\begin{equation}
E_{self}=\frac{Vk_{B}T}{2}\int\frac{d\bold{k}}{(2\pi)^3}\frac{\varkappa^2({\bold{k}})}{k^2}.
\end{equation}
$G_{\alpha\gamma}(\bold{k})$ are the Fourier-images of the structure factors of the reference system which can be calculated from the following matrix relation \cite{borue1988statistical}
\begin{equation}
G^{-1}_{\alpha\gamma}(\bold{k})=W_{\alpha\gamma}^{-1}(\bold{k})-c_{\alpha\gamma}(\bold{k}).
\end{equation}
Now, we will turn to the theory of dipolar fluids, following from the general theory formulated above. In this case, we consider the dipolar particles as pairs of charges $\pm q$.  The relation for the structure factor of the dipolar particles in the RPA takes the following form
\begin{equation}
\label{eq:matrix1}
G^{-1}\left(\bold{k}\right)=W^{-1}\left(\bold{k}\right)-C(\bold{k})=
\begin{pmatrix}
\frac{1}{\rho\left(1-g^2(\bold{k})\right)}-c_{11}(\bold{k}) & -\frac{g(\bold{k})}{\rho\left(1-g^2(\bold{k})\right)}-c_{12}(\bold{k})\\
-\frac{g(\bold{k})}{\rho\left(1-g^2(\bold{k})\right)}-c_{12}(\bold{k}) & \frac{1}{\rho\left(1-g^2(\bold{k})\right)}-c_{22}(\bold{k})\\
\end{pmatrix}
,
\end{equation}
where
\begin{equation}
\label{eq:matrix1}
C\left(\bold{k}\right)=
\begin{pmatrix}
c_{11}(\bold{k}) & c_{12}(\bold{k})\\
c_{12}(\bold{k}) & c_{22}(\bold{k})\\
\end{pmatrix}
\end{equation}
is the matrix of the Fourier-images of the direct correlation functions of the reference system, whereas the structure matrix of dipolar molecules has the following form
\begin{equation}
\label{eq:matrix1}
W\left(\bold{k}\right)=
\begin{pmatrix}
\rho & \rho g(\bold{k})\\
\rho g(\bold{k}) & \rho\\
\end{pmatrix},
\end{equation}
where
\begin{equation}
g(\bold{k})=\int d\bold{r}g(\bold{r})e^{-i\bold{k}\bold{r}}
\end{equation}
is the characteristic function corresponding to the probability distribution function $g(\bold{r})$. The screening function \cite{Budkov2018,Budkov2019,budkov2019nonlocal,budkov2019statistical,borue1988statistical} is
\begin{equation}
\varkappa^2(\bold{k})=\frac{1}{\varepsilon_0 k_{B}T}\sum\limits_{{\alpha\gamma}}q_{\alpha}q_{\gamma}G_{\alpha\gamma}(\bold{k})=\frac{2\rho q^2}{\varepsilon_0 k_{B}T}\left(1-g(\bold{k})\right)Q(\bold{k}),
\end{equation}
where
\begin{equation}
Q(\bold{k})=\frac{1-\frac{\rho}{2}\left(c_{11}(\bold{k})+
c_{22}(\bold{k})+2c_{12}(\bold{k})\right)\left(1+g(\bold{k})\right)}{1-\rho\left(c_{11}(\bold{k})+
c_{22}(\bold{k})+2c_{12}(\bold{k})g(\bold{k})\right)+\rho^2\left(1-g^2(\bold{k})\right)\Delta(\bold{k})}
\end{equation}
and
\begin{equation}
\Delta(\bold{k})=c_{11}(\bold{k})c_{22}(\bold{k})-c_{12}^2(\bold{k}).
\end{equation}

Let us consider the reference system with $c_{11}(\bold{k})=c(\bold{k})$ and $c_{22}(\bold{k})=c_{12}(\bold{k})=0$, where $c(\bold{k})$ is the direct correlation function of the hard spheres. Thus, one of the sites (site $1$) is a center of a hard sphere, while the other site (site $2$) is a point-like one which does not correlate with the sites of all the species. Essentially, such a reference system describes a set of hard spheres with a grafted point-like particle which can freely penetrate inside the hard spheres. Thus, in this case we obtain
\begin{equation}
Q(\bold{k})=1+\frac{\rho}{2}h(\bold{k})\left(1-g(\bold{k})\right),
\end{equation}
where
\begin{equation}
h(\bold{k})=\frac{c(\bold{k})}{1-\rho c(\bold{k})}
\end{equation}
is the correlation function of the hard spheres \cite{hansen1990theory}.

Further, using the following model characteristic function
\begin{equation}
g(\bold{k})=\frac{1}{1+\frac{k^2l^2}{6}},
\end{equation}
the approximation
\begin{equation}
Q(\bold{k})\approx 1+\frac{\rho}{2}h(0)\left(1-g(\bold{k})\right)=1+\frac{Z_{0}-1}{2}\left(1-g(\bold{k})\right),
\end{equation}
and taking the integral (\ref{Fcorr3}), we arrive at the following relation for the density of the electrostatic free energy
\begin{equation}
\label{Fcorr4}
f_{el}=-\frac{k_{B}T}{l^3}\Lambda(y,\alpha),
\end{equation}
where $l$ is the dipole length and the auxiliary functions
\begin{equation}
\nonumber
\Lambda(y,\alpha)=\left(1-\frac{3\alpha}{4}\right)\sigma(y)-\frac{3\sqrt{6}\left((\alpha+4)(y^2+2y+y\sqrt{1+y})+8(1+\sqrt{1+y})\right)}{8\pi\left(1+\sqrt{1+y}\right)}
\end{equation}
\begin{equation}
\label{sigma2}
+\frac{3\sqrt{6}\exp\left[\frac{\alpha y}{4(1+\sqrt{1+y})^2}\right]\left(y\left(4+\sqrt{1+y}(\alpha+2)\right)+2y^2+4(1+\sqrt{1+y})\right)}{4\pi (1+\sqrt{1+y})}
\end{equation}
and
\begin{equation}
\sigma(y) = \frac{\sqrt{6}}{4\pi}\left[2(1+y)^{3/2}-2-3y\right]
\end{equation}
are introduced. Here, $\alpha=1-Z_{0}=1-\rho k_{B}T\chi_{0}$ with the isothermal compressibility $\chi_{0}$ of the hard spheres and $y=q^2l^2\rho/3\varepsilon_0 k_{B}T$. We would like to note that with good accuracy one can use the simplified relation for the electrostatic free energy of the dipolar hard spheres fluid
\begin{equation}
F_{el}=-\frac{Vk_{B}T}{l^3}\left(1-\frac{3}{4}\alpha\right)\sigma(y).
\end{equation}
In the Percus-Yewick approximation
\begin{equation}
\label{Fhs}
F_{0}=N k_B T\left(\ln(\lambda^3\rho)-1\right)+N k_B T \left(-\ln(1 - \eta) + \frac{3\eta}{1 - \eta} + \frac{3 \eta^2}{2(1 - \eta)^2}\right),
\end{equation}
taking into account the equation of state for the reference system
\begin{equation}
 P_{0}= \rho k_B T \frac{1 + \eta + \eta^2}{(1 - \eta)^3}
\end{equation}
and the relation for the compressibility $\chi_{0}=\rho^{-1}\partial{\rho}/\partial{P_{0}}$,
one can easily obtain a relation for the $"$compressibility factor$"$
\begin{equation}
\alpha=\frac{\eta(4-\eta)(2+\eta^2)}{(1+2\eta)^2},
\end{equation}
where $\eta=\pi d^3\rho /6$ is the packing fraction of the hard spheres; $d$ is the hard sphere diameter; $\lambda$ is the thermal de Broglie wavelength.

\section{Appendix II: Pressure and chemical potential in the bulk phase}
The total pressure $P$ and chemical potential $\mu$ are the sum of four contributions:
\begin{equation}
P = \rho\frac{\partial f}{\partial\rho}-f=P_{id}+P_{ex}=P_{id}+ P_{sr}+ P_{el}
\end{equation}
and
\begin{equation}
\mu =\frac{\partial f}{\partial\rho}= \mu_{id}+\mu_{ex}=\mu_{id}+\mu_{sr}+\mu_{el}
\end{equation}
where $P_{id}=\rho k_{B}T$ and $\mu_{id}=k_{B}T\ln(\rho\lambda^3)$ are, respectively, the ideal gas pressure and chemical potential; $P_{ex}$ and $\mu_{ex}$ are the excess pressure and chemical potential, respectively, which, in turn, can be written through the sums of three contributions.

The ideal gas and short-range interaction contributions to the pressure and chemical potential are, respectively,
\begin{equation}
P_{id}+P_{sr}= \rho k_B T \frac{1 + \eta + \eta^2}{(1 - \eta)^3}+ \frac{1}{2}B\rho^2
\end{equation}
and
\begin{equation}
    \mu_{id}+\mu_{sr} = k_B T \ln(\rho\lambda^3) +  k_B T \left(-\ln(1 - \eta) +  \frac{\eta(14 - 13\eta + 5\eta^2)}{2(1 - \eta)^3} \right)+B\rho.
\end{equation}

The electrostatic contribution to the chemical potential takes the following form
\begin{equation}
\mu_{el} = -\frac{k_B T}{l^3}\left[\left(1 - \frac{3}{4}\alpha\right)\Theta_1 + \sigma(y)\Theta_2\right]
\end{equation}
with the auxiliary functions
\begin{equation}
\Theta_1 =\frac{\sqrt{6}p^2}{4 \pi\epsilon_0 k_B T}(\sqrt{1 + y} - 1),
\end{equation}
\begin{equation}
\Theta_2 = -\frac{\pi d_{BH}^3}{2} \frac{(1-\eta)^3(2+\eta)}{(1+2\eta)^3}.
\end{equation}
The electrostatic contribution to the pressure can be calculated by the relation
\begin{equation}
P_{el} = \mu_{el}\rho - f_{el}.
\end{equation}

\section{Appendix III}
This Appendix presents detailed information about the contributions to the one-particle direct correlation function for the slit geometry. The direct correlation function of the specific interactions is
\begin{equation}
c^{(1)}_{spc}(z) =  \pi \beta  \epsilon_{sw}  \int\limits_{z - \sigma_{sw}/2}^{z + \sigma_{sw}/2} dz^{\prime} \rho(z^{\prime}) (\sigma_{sw}^2/4 - (z - z^{\prime})^2)
\end{equation}
and the contribution from the WCA potential $c^{(1)}_{WCA}(z)$
\begin{equation}
c^{(1)}_{WCA}(z) =  \int\limits_{z - r_c}^{z + r_c} dz^{\prime} \rho(z^{\prime})g_{WCA}(z,z^{\prime}),
\end{equation}
where $g_{WCA}(z,z^{\prime})$ is
\[
g_{WCA}(z,z^{\prime})=
\left\{
  \begin{tabular}{ccc}
  $4\pi\epsilon\sigma^2 \psi(r_m) -\pi\epsilon(r_m^2 - (z^{\prime} - z)^2)$ & ~if~ & $|z - z^{\prime}|  < r_m$ \\
  $4\pi\epsilon\sigma^2 \psi(z^{\prime} - z)$ & ~if~ & $r_m<|z - z^{\prime}|< r_c$,\\
  $0$ & ~if~ & $|z - z^{\prime}|>r_c.$
  \end{tabular}
  \right\}
\]

Above we used the following notations $r_m = 2^{1/6}\sigma$ and $\psi(x)$ is
\begin{equation}
\psi(x) =  -\frac{1}{5}\left( \left(\frac{\sigma}{r_c}\right)^{10} - \left(\frac{\sigma}{x}\right)^{10}\right) + \frac{1}{2} \left( \left(\frac{\sigma}{r_c}\right)^{4} - \left(\frac{\sigma}{x}\right)^{4}\right).
\end{equation}

The three independent weighted functions are:
\begin{equation}
n_3(z) = \pi\int\limits_{z - R}^{z + R} dz^{\prime} \rho(z^{\prime}) (R^2 - (z - z^{\prime})^2),
\end{equation}
\begin{equation}
n_2(z) = 2\pi R \int\limits_{z - R}^{z + R} dz^{\prime} \rho(z^{\prime}),
\end{equation}
\begin{equation}
\mathbf{n}^{(v)}_2(z) = 2 \pi \mathbf{e_z} \int\limits_{z - R}^{z + R} dz \rho(z^{\prime}) (z - z^{\prime}),
\end{equation}
where $\mathbf{e_z}$ is the unit vector along the z-axis and $R = d_{BH}/2$.
Due to the fact that only three weighted functions are independent, we can express the hard spheres direct correlation function in the FMT approximation in the following way:
\begin{equation}
c^{(1)}_{fmt}(z) =  2\pi\int\limits_{z - R}^{z+R} dz^{\prime}\left[\frac{1}{2}\frac{\partial \Phi}{\partial n_3}(R^2 - (z^{\prime} - z)^2) + R\frac{\partial \Phi}{\partial n_2} + \frac{\partial \Phi}{\partial n^{(v)}_2}(z^{\prime} - z) \right],
\end{equation}
where the derivatives are determined as follows
\begin{equation}
\frac{\partial \Phi}{\partial n_3} = \frac{n_2}{4\pi R^2(1 - n_3)} + \frac{n_2^2 - (n^{(v)}_2)^2}{4\pi R (1 - n_3)^2} + \frac{n_2^3 - 3n_2 (n^{(v)}_2)^2}{12\pi(1-n_3)^3},
\end{equation}
\begin{equation}
\frac{\partial \Phi}{\partial n_2} = -\ln(1 - n_3)/(4\pi R) + \frac{n_2}{2\pi R(1 - n_3)} + \frac{n_2^2 - (n^{(v)}_2)^2}{8\pi(1-n_3)^2},
\end{equation}
\begin{equation}
\frac{\partial \Phi}{\partial n^{(v)}_2} = -\frac{n^{(v)}_2}{2\pi R(1 - n_3)} - \frac{n_2 n^{(v)}_2}{4\pi(1-n_3)^2}.
\end{equation}

The direct correlation function of electrostatic interactions is
\begin{equation}
c^{(1)}_{el}(z) =  -\beta\phi_{el}(\bar{\rho}(z)) - \frac{3\beta}{4 R_w^3}\int\limits_{-\infty}^{\infty} dz^{\prime} \rho(z^{\prime})  \left[ \frac{\mu_{el}(\bar{\rho}(z^{\prime}))}{\bar{\rho}(z^{\prime})} - \frac{\phi_{el}(\bar{\rho}(z^{\prime}))}{\bar{\rho}(z^{\prime})}\right] (R_w^2 - (z - z^{\prime})^2).
\end{equation}

\section{Appendix IV: direct correlation functions}
In this Appendix, we consider the calculations of the second direct correlation function $c^{(2)}(\bold{r},\bold{r}^{\prime})$ within the nonlocal density functional theory, considered in the main text.
The second direct correlation function $c^{(2)}(\mathbf{r} ,\mathbf{r^{\prime}})$ is the sum of the following contributions:
\begin{eqnarray}
    c^{(2)}_{el} (\mathbf{r} ,\mathbf{r^{\prime}}) &=&-   \frac{2\beta(\mu_{el}(\bar{\rho}(\mathbf{r^{\prime}}))-\phi_{el}(\bar{\rho}(\mathbf{r^{\prime}})))}{\bar{\rho}(\mathbf{r^{\prime}})} \omega_{el}(|\mathbf{r} - \mathbf{r^{\prime}}|) \nonumber \\
    &-&\int_V d\mathbf{r^{\prime\prime}} \rho(\mathbf{r^{\prime\prime}}) \left[\frac{1}{\bar{\rho}( \mathbf{r^{\prime\prime}})}\frac{\partial \beta\mu_{el}(\bar{\rho}(\mathbf{r^{\prime \prime}}))}{\partial \bar{\rho}(\mathbf{r^{\prime\prime}})}  - \frac{2\beta(\mu_{el}(\bar{\rho}(\mathbf{r^{\prime \prime}})) - \phi_{el}(\bar{\rho}(\mathbf{r^{\prime \prime}}))}{\bar{\rho}^2(\mathbf{r^{\prime \prime}})} \right]\nonumber \\ &\times& \omega_{el}(|\mathbf{r} - \mathbf{r^{\prime\prime}}|) \omega_{el}(|\mathbf{r^{\prime}} - \mathbf{r^{\prime\prime}}|), \nonumber
\end{eqnarray}
\begin{equation}
    c^{(2)}_{WCA} (\mathbf{r} ,\mathbf{r^{\prime}}) = -\beta V_{WCA}(|\mathbf{r} - \mathbf{r^{\prime}}|),
\end{equation}
\begin{equation}
    c^{(2)}_{spc} (\mathbf{r} ,\mathbf{r^{\prime}}) = -\beta V_{spc}(|\mathbf{r} - \mathbf{r^{\prime}}|),
\end{equation}
\begin{equation}
    c^{(2)}_{fmt} (\mathbf{r} ,\mathbf{r^{\prime}}) = -\beta\sum\limits_{\alpha}\sum\limits_{\gamma} \int_V  d\mathbf{r^{\prime\prime}}\frac{\partial^2 \Phi(\{n\})}{\partial n_{\alpha}(\mathbf{r^{\prime\prime}})\partial n_{\gamma}(\mathbf{r^{\prime\prime}})}\omega_{\alpha}(\mathbf{r^{\prime\prime}} - \mathbf{r})\omega_{\gamma}(\mathbf{r^{\prime\prime}} - \mathbf{r^{\prime}}).
\end{equation}

The second direct correlation function for the homogeneous water in the Fourier-representation can be written as a sum of several contributions
\begin{equation}
\rho c^{(2)}(k) = \rho (c_{py}^{(2)}(k) +  c_{spc}(k) + c_{wca}(k) + c_{el}(k)),
\end{equation}
where
\begin{equation}
\rho c_{spc}(k) = 24 \eta \epsilon_{sw} \beta \left(\frac{r_{sw}}{d_{HS}}\right)^3 \frac{\sin(kr_{sw}) - kr_{rw}\cos(kr_{sw})}{(kr_{sw})^3},
\end{equation}
\begin{eqnarray}
\rho c_{WCA}(k) &=& 24 \eta \epsilon \beta \left(\frac{r_{m}}{d_{HS}}\right)^3 \frac{\sin(kr_{m}) - kr_{m}\cos(kr_{m})}{(kr_{m})^3} \nonumber \\
    &-& 96\beta\epsilon\eta\frac{\sigma}{k d_{HS}^3} \int\limits_{r_m}^{r_c} dr \sin(kr)\left[ \left(\frac{\sigma}{r}\right)^{11} - \left(\frac{\sigma}{r}\right)^5\right],
\end{eqnarray}
and
\begin{equation}
\rho c_{el}(k) = -\beta \rho \omega_{el}^2(k)\frac{\partial \mu_{el}}{\partial \rho} - 2\beta\rho\omega_{el}(k)(1 - \omega_{el}(k))\left(\frac{\mu_{el} - \phi_{el}}{\rho}\right).
\end{equation}
$c_{py}^{(2)}(k)$ is the Fourier image of the direct correlation function of the hard spheres system in the Perkus-Yevick approximation (see, for instance, \cite{hansen1990theory}), $r_{rw} = \sigma_{rw}/2$ and the Fourier-image of smoothing function $\omega_{el}$ is:
\begin{equation}
    \omega_{el}(k) = -3 \frac{kR_w \cos(kR_w) - \sin(kR_w)}{(kR_w)^3}.
\end{equation}

redpajama_set_name: RedPajamaArXiv


MaskOn sells all styles of clothing in a variety of sizes. In order to help you better determine the size to best fit your figure, we have created the size charts below. Many outfits in our online storefront are available in multiple sizes, including plus sizes.
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You take your chest measurement, which in the above example we said 36″ and add 4″ to it.
If you have a 36″ chest, your bra size would be 40.
You would then purchase a 40D, C, DD, E or whatever cup size you chose for your breast forms. If you chose a 36D as your breast form size, you would buy a 40D bra.
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Janet's closet provides the crossdresser with a variety of clothing. You can find the skirt, dress, or outfit you've always dreamed of wearing right here. If you don't know what size to wear, simply review the sizing chart above or contact Janet and she'll help you pick out what is right for you.
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text:
Official Google Docs App For Android Is Out - It's About Time
2011/04/27 9:32am PDT Apr 27, 2011
If there is one single Google service that I've wanted on my phone since the day I got it, it's Google Docs. That wait is finally over, because Google has released an official Docs app for Android - and it's nothing short of awesome.
This app not only allows you to view and edit all of your Docs, but also brings a few other killer features. Firstly, it offers a widget that allows you to quickly create a new document, take a picture and upload it, or directly access your starred documents.
The most impressive feature, however, is the ability to snap a picture of a document and turn it into a fully editable Google doc. Just create a new Document from Photo, snap the picture, and the converted doc will show up in your list. You can also convert pictures currently saved to your Google Docs account by sharing them with the Docs app.
As always, it's free in the Market. Get it while it's hot!
Source: Google Docs Blog
google docs app
Another Day, Another Source Code Delivered: Samsung Releases The Source For The Galaxy Prevail
[Hands-On] Google Docs Photo Upload OCR: It Kind Of Sucks At This Point


"They won't bite. A biotech company called Intrexon hopes these genetically engineered #mosquitoes can help stop the spread of the Zika virus. The insects were developed mainly to fight dengue fever, but Zika is spread by the same type of insect. When the male mosquitoes are released to mate with wild females, the offspring die before reaching adulthood. Now Intrexon — which has ventures ranging from potential cancer cures to cloned kittens — needs to persuade federal agencies, foreign governments and nonprofit health organizations to place orders. It must also counter caution from the @worldhealthorganization and federal officials, who question whether the technique will be effective on a large scale. Andrew Testa photographed a worker with her hand in a cage full of genetically modified male mosquitoes." By nytimes on Instagram.


Abstract. Hydro-geomorphological risk factors that have degraded the spa tourism of Telega. After an intense exploitation of salt deposits of Telega, that are part of the faulted diapirs of external Curvature Subcarpathians, the infiltrated water resulted from rainfall and surface flow settled in the old salt mines. For more than 140 years, these waters with a high quantity of salt were used for their therapeutically qualities. In the last years, view the increase of very powerful rainfalls, the risk of producing such hydro-geomorphological processes has grown, with a direct impact on the spa tourism potential. Our thorough research foresees neither a real stabilization of these processes, nor the rehabilitation of the spa tourism for Telega.
Key words: hydro-geomorphological processes, spa tourism, Telega, Prahova Subcarpathians.


This year my mother was diagnosed with lung cancer and through it all she has remained brave while retaining all the grace and dignity of an Angel. I do not make it a practice to ask many favors of my net friends. I can't recall ever asking anyone to pray for me, however my mother believes in the power of prayer, so for my mother I ask you to pray for her, to whomever or whatever you believe in. If you don't believe in prayer please just think of her and wish her well, for the God she believes in hears all types of prayers. Please pass this along to everyone on your ICQ list or send the URL through email to anyone who might be willing to help the hit counter increase. Lets show my mom how many of us are praying for her and she can then realize what I already know, that the fine people of the net are some of the most caring people I have ever known and that together we can move mountains.
For Mothers Day if I could have any gift in the world it would be the gift of looking at the world through my mother's eyes.
Mama's eyes could see things that others eyes would miss, like seeing the trouble I'd gotten into without me saying a word.
Mama's eyes could see when I was truly sorry and the punishment I'd given myself, she said, was more than I'd deserved from her.
Mama's eyes could see my desperate want for something I didn't dare ask for, and somehow no matter how little we had, she'd find a way to give it to me.
Mama's eyes could see when I'd been picked on at school for not always' being like everyone else and in mama's arms I always seemed to fit right in.
Mama's eyes could see when I was lonely and always stopped a while to play with me no matter how busy she was.
Mama's eyes could see what was wrong with me even when I didn't know myself.
Mama's eyes could see when I was sick without me even saying so.
Mama's eyes could see the fear in me no matter how brave I acted.
Mama's eyes could see the love sick look all over my face when everyone else just thought I'd lost my senses.
Even as I grew and moved away mama's eyes seemed to be able to look at me right through the phone.
Even now, Mama's eyes are an amazing tool she uses to love and nurture her children even in adulthood.
Yes, the greatest gift I could ever receive would be the gift of seeing the world through my Mothers eyes.
Update: September 1999. Mom endured several radiation treatments before undergoing surgery to remove a Pancoast Tumor in October of 1998. I could not be with my mom so while she was in surgery I released my fears and anxiety by building her this (my very first) web page. Mom surprised most everyone including the doctors with her astounding recovery, everyone that is, except me. I guess in my eyes mom has always been a fighter, she never let me give up so the thought of her giving up never entered my mind, though it probably entered hers. At her 6 month check up mom was deemed 'Cancer FREE'. She will still go for her check ups (won't you mom? *S*) but the future looks very good and my every prayer has been answered.
Update: September 2000: Mom had another check up in August, 2000. All the tests have come back clear...YES!!! WAY TO GO MOM! Mom continues to be the wonderful woman she has always been but I do believe I see a little more 'stopping to smell the roses' in her life. She always taught me that life was precious but now I think she understands that in a way only others who have been through what she has can really understand.
Click on the letter to Email my Mom!


text:
MPC NY Teams Up with The Sherry Company to Take Tromba on a Surreal Journey
Creative Director Andrew Montague of MPC Creative has earned a coveted Young Director Award nomination, having recently teamed up with agency The Sherry Company to create a beautiful film for Tequila Tromba. 'Tromba Journey' is a CG adventure that follows the tequila's production process via finely rendered floating islands representing every step between the Jalisco Mountains and the shining cities of the world.
[jwplayer mediaid="9062″]
"This project was an exciting opportunity to tell the Tromba story and create a world and mythology around the brand itself," explains Montague. "I wanted to capture the intimate scale of Tromba's operations as well as their authentic approach to making tequila. By connecting each floating world to the other via a waterfall, a barrel and a plane, we could flow smoothly and follow the journey of Tromba from beginning to end."
The Sherry Company Producer James Sherry recalls, "When we started the Tromba spot, I explained to Andrew our plan to change people's perceptions of tequila by promoting the highlands. We talked about the culture and beautiful landscape of the region, and it was then that we formed the idea for this spot. MPC did an incredible job of bringing our collective vision to life."
The results of the Young Director Awards 2013 will be announced during the Cannes Lions Festival.
Brand: Tequila Tromba
Spot Title: "Tromba Journey" (:30)
Agency: The Sherry Company
Producer: James Sherry
Production Company: MPC Creative
Creative Director: Andrew Montague
Managing Director: Justin Lane
Executive Producer: Justin Brukman
2D Animators: Graeme Revell, Jacob Fradkin
2D Compositors: Carl Fong, Sang Lee
3D Supervisor: Dean Robinson
3D Leads: Andres Weber, Corey Langelotti
Music and Sound Design: Silencio
Executive Producer: Gin Welsh
Composer and Sound Design: Jeremy Yang and Piers Burbrook De Vere
About MPC:
MPC is a creative studio
We craft spectacular visual experiences in any space, on any screen.
We have been one of the global leaders in VFX for over 25 years, with industry-leading facilities in London, Vancouver, Los Angeles, New York and Bangalore.
Renowned for adding visual wonder and creative expertise to the advertising, film and entertainment industries, some of our most famous projects include blockbuster movies such as the "Harry Potter" franchise, "Pirates of the Caribbean: On Stranger Tides," "Prometheus" and "Life of Pi," and famous advertising campaigns for brands such as Evian, Cadbury, Sony, Coca Cola and John Lewis.
Our broad range of skill-sets provide a multitude of creative solutions, including concept design, pre-viz, shoot supervision, 2D compositing, 3D/CG effects, animation, motion design, software development, digital and experiential production, colour grading for advertising and any combination of these services.
MPC is the sum of the parts: creative partners and a range of creative solutions harnessed through a dedication to collaboration. It all comes together in our enthusiastic and talented people, working every day to be a part of creating some of the best and most inspirational work in the industry.
MPC is a Technicolor company.


I was hoping I could send this post out a bit earlier in January as it is on goal-setting, and as I am a bit anti-goal-setting at this time. I found this hilarious audio and had to share it with you. Hope you think it's funny, too!
in case vid doesn't show up, try this link.
Sir Marcus Browning: My Lord Mayor, my Lady Mayoress. My lords, ladies and gentlemen. There comes a time when we must all stand up and be counted. I am therefore standing up now and can be counted. One. To each of you I say you are a one. And ones are about to become singularly important. Because Britain is facing the gravest economic crisis since 1380. And you know many of us still remember that day. The eternal torment, worry, exasperation and all manner of (?). And if we are to quit the lights go out on our lives once more (?), we must ask ourselves crucial questions.
How do we want to get to where we want to go?
How far do we have to go before we get to where we want to be?
How would we know where we were when we got there?
HAVE WE GOT A MAP?
Why did we leave places to get to where we are?
Where were we before that we had to leave to get to where we before we knew we're going to go to where we want to be?
Where would we end up if we had the choice?
Where would we end up if we didn't have the choice?
What would we choose given the choice?
Do we have that choice to choose?
Or indeed can we be choosy about the choice choosings?
What are the choosings? Choices!
Or do we want to go right back to the beginning and start all over again.
But surely you can see my point.
Because what I'm talking about is life.
Because life is one of those things that most of us find it very difficult to avoid.
In the words of (?) "life is uncertain."
My life certainly has a certain uncertainty about it.
And I'm certain yours does too.
So with my uncertainty and your uncertainty there's certainly a certain degree of uncertainty about, of that we can be quite sure.
So let's buckle down, shall we?
Because we don't want to end up, do we?
Like the blind man in the dark room looking for the black cat that isn't there.
It's important to take ourselves lightly once in awhile, don't you think? Happy Goal-Setting!


text:
package dairyclient

import (
	"bytes"
	"encoding/json"
	"errors"
	"io/ioutil"
	"math"
	"net/http"
	"net/url"
	"testing"

	"github.com/dairycart/dairycart/models/v1"

	"github.com/stretchr/testify/assert"
)

func TestClientError(t *testing.T) {
	t.Run("with error", func(*testing.T) {
		expected := "arbitrary error"
		ce := &ClientError{Err: errors.New(expected)}
		assert.Equal(t, expected, ce.Error(), "expected and actual error messages should be equal")
	})

	t.Run("with API error", func(*testing.T) {
		expected := "arbitrary error"
		ce := &ClientError{FromAPI: &models.ErrorResponse{Message: expected}}
		assert.Equal(t, expected, ce.Error(), "expected and actual error messages should be equal")
	})

	t.Run("without error", func(*testing.T) {
		ce := &ClientError{}
		assert.Empty(t, ce.Error())
	})
}

func TestMapToQueryValues(t *testing.T) {
	exampleQueryParams := map[string]string{
		"param": "value",
	}

	expected := url.Values{
		"param": []string{"value"},
	}
	actual := mapToQueryValues(exampleQueryParams)

	assert.Equal(t, expected, actual, "expected and actual url values should be equal")
}

type testNormalStruct struct {
	Thing string `json:"thing"`
}

type testFailReader struct{}

func (ft testFailReader) Read([]byte) (int, error) {
	return 0, errors.New("pineapple on pizza")
}

func TestUnmarshalBody(t *testing.T) {
	t.Run("normal operation", func(*testing.T) {
		exampleInput := &http.Response{
			StatusCode: http.StatusOK,
			Body: ioutil.NopCloser(bytes.NewBufferString(`{"thing":"something"}`)),
		}

		expected := testNormalStruct{Thing: "something"}
		actual := testNormalStruct{}
		err := unmarshalBody(exampleInput, &actual)

		assert.Nil(t, err)
		assert.Equal(t, expected, actual, "expected and actual unmarshaled structs should match")
	})

	t.Run("should fail when receiving nil", func(*testing.T) {
		exampleFailureInput := &http.Response{
			StatusCode: http.StatusOK,
			Body: ioutil.NopCloser(testFailReader{}),
		}

		err := unmarshalBody(exampleFailureInput, nil)
		assert.NotNil(t, err)
		expected := &ClientError{Err: errors.New("unmarshalBody cannot accept nil values")}
		assert.Equal(t, expected, err, "expected error string %s")
	})

	t.Run("fails when it receives a non pointer", func(*testing.T) {
		exampleFailureInput := &http.Response{
			StatusCode: http.StatusOK,
			Body: ioutil.NopCloser(testFailReader{}),
		}

		err := unmarshalBody(exampleFailureInput, testNormalStruct{})
		assert.NotNil(t, err)
		expected := &ClientError{Err: errors.New("unmarshalBody can only accept pointers")}
		assert.Equal(t, expected, err)
	})

	t.Run("returns ReadAll error", func(*testing.T) {
		exampleFailureInput := &http.Response{
			StatusCode: http.StatusOK,
			Body: ioutil.NopCloser(testFailReader{}),
		}

		err := unmarshalBody(exampleFailureInput, &testNormalStruct{})
		assert.NotNil(t, err)
	})

	t.Run("with invalid struct", func(*testing.T) {
		exampleInput := &http.Response{
			StatusCode: http.StatusOK,
			Body: ioutil.NopCloser(bytes.NewBufferString(`{"invalid_lol}`)),
		}

		actual := testNormalStruct{}
		err := unmarshalBody(exampleInput, &actual)

		assert.NotNil(t, err)
	})
}

func TestConvertIDToString(t *testing.T) {
	testCases := []struct {
		input    uint64
		expected string
	}{
		{
			0,
			"0",
		},
		{
			123,
			"123",
		},
		{
			math.MaxUint64,
			"18446744073709551615",
		},
	}

	for _, tc := range testCases {
		actual := convertIDToString(tc.input)
		assert.Equal(t, tc.expected, actual, "converIDToString failed: expected %s, got %s", tc.expected, actual)
	}
}

type testBreakableStruct struct {
	Thing json.Number `json:"thing"`
}

func TestCreateBodyFromStruct(t *testing.T) {
	t.Run("normal operation", func(*testing.T) {

		in := testNormalStruct{Thing: "something"}
		_, err := createBodyFromStruct(in)
		assert.Nil(t, err)
	})

	t.Run("with invalid input", func(*testing.T) {

		f := &testBreakableStruct{Thing: "dongs"}
		_, err := createBodyFromStruct(f)
		assert.NotNil(t, err)
	})
}

redpajama_set_name: RedPajamaGithub