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\documentclass[aps,endfloats*,preprint,amssymb]{revtex4} |
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\usepackage{times} |
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\usepackage{mathptm} |
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\begin{document} |
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\renewcommand{\thefootnote}{\fnsymbol{footnote}} |
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\renewcommand{\theequation}{\arabic{section}.\arabic{equation}} |
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\bibliographystyle{pccp} |
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\title{Symmetry breaking and the $P_{\beta'}$ Ripple phase} |
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\author{Xiuquan Sun and J. Daniel Gezelter} |
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\email[]{E-mail: gezelter@nd.edu} |
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\affiliation{Department of Chemistry and Biochemistry,\\ |
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University of Notre Dame, \\ |
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Notre Dame, Indiana 46556} |
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\date{\today} |
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\begin{abstract} |
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The ripple phase in phosphatidylcholine (PC) bilayers has never been |
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completely explained. We present a simple (XYZ) spin-lattice model |
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that allows spins to vary their elevation as well as their |
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orientation. The extra degree of freedom allows hexagonal lattices of |
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spins to find states that break out of the normally frustrated |
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randomized states and are stabilized by long-range antiferroelectric |
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ordering. To break out of the frustrated states, the spins must form |
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``rippled'' phases that make the lattices effectively |
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non-hexagonal. Our XYZ model contains a hydrophobic interaction and |
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dipole-dipole interactions to describe the interaction potential for |
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model lipid molecules. We find non-thermal ripple phases and note |
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that the wave vectors for the ripples are always perpendicular to the |
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director axis for the dipoles. Non-hexagonal lattices of dipoles are |
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not inherently frustrated, and are therefore less likely to form |
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ripple phases because they can easily form low-energy |
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antiferroelectric states. We see that the dipolar order-disorder |
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transition is substantially lower for hexagonal lattices and that the |
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ordered phase for this lattice is clearly rippled. |
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\end{abstract} |
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\maketitle |
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\section{Introduction} |
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\label{Int} |
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Fully hydrated lipids will aggregate spontaneously to form bilayers |
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which exhibit a variety of phases depending on their temperatures and |
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compositions. Among these phases, a periodic rippled phase |
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($P_{\beta'}$) appears as an intermediate phase between the gel |
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($L_\beta$) and fluid ($L_{\alpha}$) phases for relatively pure |
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phosphatidylcholine (PC) bilayers. The ripple phase has attracted |
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substantial experimental interest over the past 30 years. Most |
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structural information of the ripple phase has been obtained by the |
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X-ray diffraction~\cite{Sun96,Katsaras00} and freeze-fracture electron |
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microscopy (FFEM).~\cite{Copeland80,Meyer96} Recently, Kaasgaard {\it |
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et al.} used atomic force microscopy (AFM) to observe ripple phase |
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morphology in bilayers supported on mica.~\cite{Kaasgaard03} The |
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experimental results provide strong support for a 2-dimensional |
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hexagonal packing lattice of the lipid molecules within the ripple |
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phase. This is a notable change from the observed lipid packing |
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within the gel phase.~\cite{Cevc87} |
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|
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A number of theoretical models have been presented to explain the |
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formation of the ripple phase. Marder {\it et al.} used a |
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curvature-dependent Landau-de Gennes free-energy functional to predict |
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a rippled phase.~\cite{Marder84} This model and other related continuum |
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models predict higher fluidity in convex regions and that concave |
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portions of the membrane correspond to more solid-like regions. |
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Carlson and Sethna used a packing-competition model (in which head |
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groups and chains have competing packing energetics) to predict the |
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formation of a ripple-like phase. Their model predicted that the |
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high-curvature portions have lower-chain packing and correspond to |
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more fluid-like regions. Goldstein and Leibler used a mean-field |
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approach with a planar model for {\em inter-lamellar} interactions to |
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predict rippling in multilamellar phases.~\cite{Goldstein88} McCullough |
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and Scott proposed that the {\em anisotropy of the nearest-neighbor |
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interactions} coupled to hydrophobic constraining forces which |
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restrict height differences between nearest neighbors is the origin of |
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the ripple phase.~\cite{McCullough90} Lubensky and MacKintosh |
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introduced a Landau theory for tilt order and curvature of a single |
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membrane and concluded that {\em coupling of molecular tilt to membrane |
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curvature} is responsible for the production of |
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ripples.~\cite{Lubensky93} Misbah, Duplat and Houchmandzadeh proposed |
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that {\em inter-layer dipolar interactions} can lead to ripple |
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instabilities.~\cite{Misbah98} Heimburg presented a {\em coexistence |
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model} for ripple formation in which he postulates that fluid-phase |
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line defects cause sharp curvature between relatively flat gel-phase |
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regions.~\cite{Heimburg00} Kubica has suggested that a lattice model of |
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polar head groups could be valuable in trying to understand bilayer |
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phase formation.~\cite{Kubica02} Bannerjee used Monte Carlo simulations |
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of lamellar stacks of hexagonal lattices to show that large headgroups |
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and molecular tilt with respect to the membrane normal vector can |
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cause bulk rippling.~\cite{Bannerjee02} |
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Large-scale molecular dynamics simulations have also been performed on |
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rippled phases using united atom as well as molecular scale |
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models. De~Vries {\it et al.} studied the structure of lecithin ripple |
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phases via molecular dynamics and their simulations seem to support |
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the coexistence models (i.e. fluid-like chain dynamics was observed in |
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the kink regions).~\cite{deVries05} Ayton and Voth have found |
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significant undulations in zero-surface-tension states of membranes |
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simulated via dissipative particle dynamics, but their results are |
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consistent with purely thermal undulations.~\cite{Ayton02} Brannigan, |
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Tamboli and Brown have used a molecular scale model to elucidate the |
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role of molecular shape on membrane phase behavior and |
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elasticity.~\cite{Brannigan04b} They have also observed a buckled hexatic |
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phase with strong tail and moderate alignment attractions.~\cite{Brannigan04a} |
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Ferroelectric states (with long-range dipolar order) can be observed |
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in dipolar systems with non-hexagonal packings. However, {\em |
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hexagonally}-packed 2-D dipolar systems are inherently frustrated and |
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one would expect a dipolar-disordered phase to be the lowest free |
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energy configuration. Concomitantly, it would seem unlikely that a |
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frustrated lattice in a dipolar-disordered state could exhibit the |
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long-range periodicity in the range of 100-600 \AA (as exhibited in |
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the ripple phases studied by Kaasgard {\it et al.}).~\cite{Kaasgaard03} |
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The various theoretical models have attributed membrane rippling to |
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various causes which appear contradictory. We are left with a number |
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of open questions: 1) Are inter-layer interactions required to explain |
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the ripple, or can a single bilayer (or even a single leaf) exhibit |
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the rippling? 2) To what degree is the dipolar anisotropy of the head |
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group important in determining the rippling? 3) Is chain fluidity |
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required? (i.e. are the coexistence models necessary to explain the |
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ripple phenomenon?) 4) How could a state with long-range order be |
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formed using a substrate consisting of 2-D hexagonally-packed dipolar |
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molecules? What we present here is an attempt to find the simplest |
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model which will exhibit this phenomenon. We are using a very simple |
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modified XYZ lattice model; details of the model can be found in |
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section \ref{sec:model}, results of Monte Carlo simulations using this |
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model are presented in section |
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\ref{sec:results}, and section \ref{sec:discussion} contains our conclusions. |
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\section{The Web-of-Dipoles Model} |
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\label{sec:model} |
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The model used in our simulations is shown schematically in |
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Figs. \ref{fmod1} and \ref{fmod2}. |
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\begin{figure}[ht] |
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\centering |
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\caption{The modified X-Y-Z model used in our simulations. Point dipoles are |
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represented as arrows. Dipoles are locked to the lattice points in x-y |
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plane and connect to their nearest neighbors with harmonic |
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potentials. The lattice parameters $a$ and $b$ are indicated above.} |
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\includegraphics[width=\linewidth]{picture/WebOfDipoles.eps} |
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\label{fmod1} |
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\end{figure} |
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|
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\begin{figure}[ht] |
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\centering |
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\caption{The 6 coordinates describing the state of a 2-dipole system |
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in our extended X-Y-Z model. $z_i$ is the height of dipole $i$ from |
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an arbitrary x-y plane, $\theta_i$ is the angle that the dipole makes |
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with the laboratory z-axis and $\phi_i$ is the angle between |
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the projection of the dipole on x-y plane with the x axis.} |
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\includegraphics[width=\linewidth]{picture/xyz.eps} |
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\label{fmod2} |
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\end{figure} |
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In this model, lipid molecules are represented by point-dipoles (which |
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is a reasonable approximation to the zwitterionic head groups of the |
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phosphatidylcholine head groups). The dipoles are locked in place to |
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their original lattice sites on the x-y plane. The original lattice |
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may be either hexagonal ($a/b = \sqrt{3}$) or non-hexagonal. However, |
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each dipole has 3 degrees of freedom. They may move freely {\em out} of the |
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x-y plane (along the $z$ axis), and they have complete orientational |
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freedom ($0 <= \theta <= \pi$, $0 <= \phi < 2 \pi$). This is a |
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modified X-Y-Z model with translational freedom along the z-axis. |
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The potential energy of the system, |
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\begin{equation} |
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V = \sum_i \left[ \sum_{j>i} V^{\mathrm{dd}}_{ij} + \frac{1}{2}\sum_{j |
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\in NN_i}^6 V^{\mathrm{harm}}_{ij} \right] |
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\end{equation} |
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The dipolar head groups interact via a traditional point-dipolar |
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electrostatic potential, |
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\begin{equation} |
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V^{\mathrm{dd}}_{ij} = \frac{|\mu|^2}{4\pi \epsilon_0 r_{ij}^3} \left[ |
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{\mathbf{\hat u}_i} \cdot {\mathbf{\hat u}_j} - |
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3({\mathbf{\hat u}_i} \cdot {\mathbf{\hat |
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r}_{ij}})({\mathbf{\hat u}_j} \cdot {\mathbf{\hat r}_{ij}}) |
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\right], |
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\label{eq:vdd} |
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\end{equation} |
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and the hydrophobic interactions are approximated with a nearest |
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neighbor sum of harmonic interactions, |
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\begin{equation} |
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V^{\mathrm{harm}}_{ij} = \frac{k_r}{2} \left(r_{ij}-r_0\right)^2 |
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\end{equation} |
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In these potentials, $\mathbf{\hat u}_i$ is the unit vector pointing |
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along dipole $i$ and $\mathbf{\hat r}_{ij}$ is the unit vector |
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pointing along the inter-dipole vector $\mathbf{r}_{ij}$. The entire |
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potential is governed by three parameters, the dipolar strength |
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($\mu$), the harmonic spring constant ($k_r$) and the preferred |
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intermolecular spacing ($r_0$). In practice, we set the value of |
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$r_0$ to the average inter-molecular spacing from the planar lattice, |
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yielding a potential model that has only two parameters for a |
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particular choice of lattice constants $a$ (along the $x$-axis) and $b$ |
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(along the $y$-axis). |
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To investigate the phase behavior of this model, we have performed a |
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series of Metropolis Monte Carlo simulations of moderately-sized (24 |
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nm on a side) patches of membrane hosted on both hexagonal ($\gamma = |
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a/b = \sqrt{3}$) and non-hexagonal ($\gamma \neq \sqrt{3}$) lattices. |
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The linear extent of one edge of the monolayer was $20 a$ and the |
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system was kept roughly square. The average distance that coplanar |
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dipoles were positioned from their six nearest neighbors was $7$ \AA. |
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Typical system sizes were 1360 lipids for the hexagonal lattices and |
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840-2800 lipids for the non-hexagonal lattices. Periodic boundary |
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conditions were used, and the cutoff for the dipole-dipole interaction |
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was set to 30 \AA. All parameters ($T$, $\mu$, $k_r$, $\gamma$) were |
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varied systematically to study the effects of these parameters on the |
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formation of ripple-like phases. |
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\section{Results and Analysis} |
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\label{sec:results} |
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\subsection{Dipolar Ordering and Coexistence Temperatures} |
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The principal method for observing the orientational ordering |
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transition in dipolar systems is the $P_2$ order parameter (defined as |
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$1.5 \times \lambda_{max}$, where $\lambda_{max}$ is the largest |
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eigenvalue of the matrix, |
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\begin{equation} |
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{\mathsf{S}} = \frac{1}{N} \sum_i \left( |
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\begin{array}{ccc} |
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u^{x}_i u^{x}_i-\frac{1}{3} & u^{x}_i u^{y}_i & u^{x}_i u^{z}_i \\ |
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u^{y}_i u^{x}_i & u^{y}_i u^{y}_i -\frac{1}{3} & u^{y}_i u^{z}_i \\ |
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u^{z}_i u^{x}_i & u^{z}_i u^{y}_i & u^{z}_i u^{z}_i -\frac{1}{3} |
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\end{array} \right). |
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\label{eq:opmatrix} |
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\end{equation} |
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Here $u^{\alpha}_i$ is the $\alpha=x,y,z$ component of the unit vector |
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for dipole $i$. $P_2$ will be $1.0$ for a perfectly-ordered system |
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and near $0$ for a randomized system. Note that this order parameter |
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is {\em not} equal to the polarization of the system. For example, |
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the polarization of the perfect antiferroelectric system is $0$, but |
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$P_2$ for an antiferroelectric system is $1$. The eigenvector of |
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$\mathsf{S}$ corresponding to the largest eigenvalue is familiar as |
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the director axis, which can be used to determine a priveleged dipolar |
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axis for dipole-ordered systems. Fig. \ref{t-op} shows the values of |
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$P_2$ as a function of temperature for both hexagonal ($\gamma = |
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1.732$) and non-hexagonal ($\gamma=1.875$) lattices. |
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|
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\begin{figure}[ht] |
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\centering |
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\caption{The $P_2$ dipolar order parameter as a function of |
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temperature for both hexagonal ($\gamma = 1.732$) and non-hexagonal |
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($\gamma = 1.875$) lattices} |
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\includegraphics[width=\linewidth]{picture/t-orderpara.eps} |
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\label{t-op} |
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\end{figure} |
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|
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There is a clear order-disorder transition in evidence from this data. |
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Both the hexagonal and non-hexagonal lattices have dipolar-ordered |
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low-temperature phases, and orientationally-disordered high |
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temperature phases. The coexistence temperature for the hexagonal |
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lattice is significantly lower than for the non-hexagonal lattices, |
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and the bulk polarization is approximately $0$ for both dipolar |
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ordered and disordered phases. This gives strong evidence that the |
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dipolar ordered phase is antiferroelectric. We have repeated the |
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Monte Carlo simulations over a wide range of lattice ratios ($\gamma$) |
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to generate a dipolar order/disorder phase diagram. Fig. \ref{phase} |
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shows that the hexagonal lattice is a low-temperature cusp in the |
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$T-\gamma$ phase diagram. |
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|
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\begin{figure}[ht] |
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\centering |
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\caption{The phase diagram for the web-of-dipoles model. The line |
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denotes the division between the dipolar ordered (antiferroelectric) |
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and disordered phases. An enlarged view near the hexagonal lattice is |
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shown inset.} |
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\includegraphics[width=\linewidth]{picture/phase.eps} |
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\label{phase} |
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\end{figure} |
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|
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This phase diagram is remarkable in that it shows an antiferroelectric |
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phase near $\gamma=1.732$ where one would expect lattice frustration |
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to result in disordered phases at all temperatures. Observations of |
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the configurations in this phase show clearly that the system has |
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accomplished dipolar orderering by forming large ripple-like |
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structures. We have observed antiferroelectric ordering in all three |
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of the equivalent directions on the hexagonal lattice, and the dipoles |
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have been observed to organize perpendicular to the membrane normal |
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(in the plane of the membrane). It is particularly interesting to |
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note that the ripple-like structures have also been observed to |
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propagate in the three equivalent directions on the lattice, but the |
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{\em direction of ripple propagation is always perpendicular to the |
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dipole director axis}. A snapshot of a typical antiferroelectric |
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rippled structure is shown in Fig. \ref{fig:snapshot}. |
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|
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\begin{figure}[ht] |
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\centering |
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\caption{Top and Side views of a representative configuration for the |
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dipolar ordered phase supported on the hexagonal lattice. Note the |
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antiferroelectric ordering and the long wavelength buckling of the |
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membrane. Dipolar ordering has been observed in all three equivalent |
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directions on the hexagonal lattice, and the ripple direction is |
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always perpendicular to the director axis for the dipoles.} |
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\includegraphics[width=\linewidth]{picture/snapshot.eps} |
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\label{fig:snapshot} |
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\end{figure} |
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|
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\subsection{Discriminating Ripples from Thermal Undulations} |
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In order to be sure that the structures we have observed are actually |
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a rippled phase and not merely thermal undulations, we have computed |
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the undulation spectrum, |
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\begin{equation} |
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h(\vec{q}) = A^{-1/2} \int d\vec{r} |
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|
h(\vec{r}) e^{-i \vec{q}\cdot\vec{r}} |
312 |
|
|
\end{equation} |
313 |
|
|
where $h(\vec{r})$ is the height of the membrane at location $\vec{r} |
314 |
|
|
= (x,y)$.~\cite{Safran94} In simple (and more complicated) elastic |
315 |
|
|
continuum models, Brannigan {\it et al.} have shown that in the $NVT$ |
316 |
|
|
ensemble, the absolute value of the undulation spectrum can be |
317 |
|
|
written, |
318 |
|
|
\begin{equation} |
319 |
|
|
\langle | h(q)|^2 \rangle_{NVT} = \frac{k_B T}{k_c |\vec{q}|^4 + |
320 |
|
|
\tilde{\gamma}|\vec{q}|^2}, |
321 |
|
|
\label{eq:fit} |
322 |
|
|
\end{equation} |
323 |
|
|
where $k_c$ is the bending modulus for the membrane, and |
324 |
|
|
$\tilde{\gamma}$ is the mechanical surface |
325 |
|
|
tension.~\cite{Brannigan04b} |
326 |
|
|
|
327 |
|
|
The undulation spectrum is computed by superimposing a rectangular |
328 |
|
|
grid on top of the membrane, and by assigning height ($h(\vec{r})$) |
329 |
|
|
values to the grid from the average of all dipoles that fall within a |
330 |
|
|
given $\vec{r}+d\vec{r}$ grid area. Empty grid pixels are assigned |
331 |
|
|
height values by interpolation from the nearest neighbor pixels. A |
332 |
|
|
standard 2-d Fourier transform is then used to obtain $\langle | |
333 |
|
|
h(q)|^2 \rangle$. |
334 |
|
|
|
335 |
|
|
The systems studied in this paper have relatively small bending moduli |
336 |
|
|
($k_c$) and relatively large mechanical surface tensions |
337 |
|
|
($\tilde{\gamma}$). In practice, the best fits to our undulation |
338 |
|
|
spectra are obtained by approximating the value of $k_c$ to 0. In |
339 |
|
|
Fig. \ref{fig:fit} we show typical undulation spectra for two |
340 |
|
|
different regions of the phase diagram along with their fits from the |
341 |
|
|
Landau free energy approach (Eq. \ref{eq:fit}). In the |
342 |
|
|
high-temperature disordered phase, the Landau fits can be nearly |
343 |
|
|
perfect, and from these fits we can estimate the bending modulus and |
344 |
|
|
the mechanical surface tension. |
345 |
|
|
|
346 |
|
|
For the dipolar-ordered hexagonal lattice near the coexistence |
347 |
|
|
temperature, however, we observe long wavelength undulations that are |
348 |
|
|
far outliers to the fits. That is, the Landau free energy fits are |
349 |
|
|
well within error bars for all other points, but can be off by {\em |
350 |
|
|
orders of magnitude} for a few (but not all) low frequency |
351 |
|
|
components. |
352 |
|
|
|
353 |
|
|
We interpret these outliers as evidence that these low frequency modes |
354 |
|
|
are {\em non-thermal undulations} which is clear evidence that we are |
355 |
|
|
actually seeing a rippled phase developing in this model system. |
356 |
|
|
|
357 |
|
|
\begin{figure}[ht] |
358 |
gezelter |
2143 |
\centering |
359 |
gezelter |
3006 |
\caption{Evidence that the observed ripples are {\em not} thermal |
360 |
|
|
undulations is obtained from the 2-d fourier transform $\langle |
361 |
|
|
|h(\vec{q})|^2 \rangle$ of the height profile ($\langle h(x,y) |
362 |
|
|
\rangle$). Rippled samples show low-wavelength peaks that are |
363 |
|
|
outliers on the Landau free energy fits. Samples exhibiting only |
364 |
|
|
thermal undulations fit Eq. \ref{eq:fit} remarkably well.} |
365 |
|
|
\includegraphics[width=\linewidth]{picture/fit.eps} |
366 |
|
|
\label{fig:fit} |
367 |
xsun |
2138 |
\end{figure} |
368 |
gezelter |
2143 |
|
369 |
gezelter |
3006 |
\subsection{Effects of Parameters on Ripple Amplitude and Wavelength} |
370 |
gezelter |
2143 |
|
371 |
gezelter |
3006 |
We have used two different methods to estimate the amplitude and |
372 |
|
|
periodicity of the ripples. The first method requires projection of |
373 |
|
|
the ripples onto a one dimensional rippling axis. Since the rippling |
374 |
|
|
is always perpendicular to the dipole director axis, we can define a |
375 |
|
|
ripple vector as follows. The largest eigenvector, $s_1$, of the |
376 |
|
|
$\mathsf{S}$ matrix in Eq. \ref{eq:opmatrix} is projected onto a |
377 |
|
|
planar director axis, |
378 |
|
|
\begin{equation} |
379 |
|
|
\vec{d} = \left(\begin{array}{c} |
380 |
|
|
\vec{s}_1 \cdot \hat{i} \\ |
381 |
|
|
\vec{s}_1 \cdot \hat{j} \\ |
382 |
|
|
0 |
383 |
|
|
\end{array} \right). |
384 |
|
|
\end{equation} |
385 |
|
|
($\hat{i}$, $\hat{j}$ and $\hat{k}$ are unit vectors along the $x$, |
386 |
|
|
$y$, and $z$ axes, respectively.) The rippling axis is in the plane of |
387 |
|
|
the membrane and is perpendicular to the planar director axis, |
388 |
|
|
\begin{equation} |
389 |
|
|
\vec{q}_{\mathrm{rip}} = \vec{d} \times \hat{k} |
390 |
|
|
\end{equation} |
391 |
|
|
We can then find the height profile of the membrane along the ripple |
392 |
|
|
axis by projecting heights of the dipoles to obtain a one-dimensional |
393 |
|
|
height profile, $h(q_{\mathrm{rip}})$. Ripple wavelengths can be |
394 |
|
|
estimated from the largest non-thermal low-frequency component in the |
395 |
|
|
fourier transform of $h(q_{\mathrm{rip}})$. Amplitudes can be |
396 |
|
|
estimated by measuring peak-to-trough distances in |
397 |
|
|
$h(q_{\mathrm{rip}})$ itself. |
398 |
|
|
|
399 |
|
|
A second, more accurate, and simpler method for estimating ripple |
400 |
|
|
shape is to extract the wavelength and height information directly |
401 |
|
|
from the largest non-thermal peak in the undulation spectrum. For |
402 |
|
|
large-amplitude ripples, the two methods give similar results. The |
403 |
|
|
one-dimensional projection method is more prone to noise (particularly |
404 |
|
|
in the amplitude estimates for the non-hexagonal lattices). We report |
405 |
|
|
amplitudes and wavelengths taken directly from the undulation spectrum |
406 |
|
|
below. |
407 |
|
|
|
408 |
|
|
In the hexagonal lattice ($\gamma = \sqrt{3}$), the rippling is |
409 |
|
|
observed from $150-300$ K. The wavelength of the ripples is |
410 |
|
|
remarkably stable at 150~\AA~for all but the temperatures closest to |
411 |
|
|
the order-disorder transition. At 300 K, the wavelength drops to 120 |
412 |
|
|
\AA. |
413 |
|
|
|
414 |
|
|
The dependence of the amplitude on temperature is shown in |
415 |
|
|
Fig. \ref{fig:t-a}. The rippled structures shrink smoothly as the |
416 |
|
|
temperature rises towards the order-disorder transition. The |
417 |
|
|
wavelengths and amplitudes we observe are surprisingly close to the |
418 |
|
|
$\Lambda / 2$ phase observed by Kaasgaard {\it et al.} in their work |
419 |
|
|
on PC-based lipids,\cite{Kaasgaard03} although this may be |
420 |
|
|
coincidental agreement given our choice of parameters. |
421 |
|
|
|
422 |
|
|
\begin{figure}[ht] |
423 |
gezelter |
2143 |
\centering |
424 |
gezelter |
3006 |
\caption{ The amplitude $A$ of the ripples vs. temperature for a |
425 |
|
|
hexagonal lattice.} |
426 |
|
|
\includegraphics[width=\linewidth]{picture/t-a-error.eps} |
427 |
|
|
\label{fig:t-a} |
428 |
xsun |
2138 |
\end{figure} |
429 |
gezelter |
2143 |
|
430 |
gezelter |
3006 |
The ripples can be made to disappear by increasing the internal |
431 |
|
|
surface tension (i.e. by increasing $k_r$). In Fig. \ref{fig:kr-a} |
432 |
|
|
we show the ripple amplitude as a function of the internal spring |
433 |
|
|
constant for non-dipolar part of the lipid interaction potential. |
434 |
|
|
Weaker ``hydrophobic'' interactions allow the lipid structure to be |
435 |
|
|
dominated by the dipoles, and stronger ``hydrophobic'' interactions |
436 |
|
|
result in much flatter membranes. Section \ref{sec:discussion} |
437 |
|
|
contains further discussion of this effect. |
438 |
xsun |
2138 |
|
439 |
gezelter |
3006 |
\begin{figure}[ht] |
440 |
|
|
\centering |
441 |
|
|
\caption{The amplitude $A$ of the ripples vs. the harmonic binding |
442 |
|
|
constant $k_r$ for both the hexagonal lattice (circles) and |
443 |
|
|
non-hexagonal lattice (squares). In both simulations the dipole |
444 |
|
|
strength ($\mu$) was 7 Debye and the temperature was 260K.} |
445 |
|
|
\includegraphics[width=\linewidth]{picture/k-a-error.eps} |
446 |
|
|
\label{fig:kr-a} |
447 |
|
|
\end{figure} |
448 |
xsun |
2138 |
|
449 |
gezelter |
3006 |
The amplitude of the ripples depends critically on the strength of the |
450 |
|
|
dipole moments ($\mu$) in Eq. \ref{eq:vdd}. If the dipoles are |
451 |
|
|
weakened substantially (below $\mu$ = 5 Debye) at a fixed temperature |
452 |
|
|
of 230 K, the membrane loses dipolar ordering and the ripple |
453 |
|
|
structures. The ripples reach a peak amplitude |
454 |
|
|
of 26~\AA~at a dipolar strength of 9 Debye. We show the dependence of |
455 |
|
|
ripple amplitude on the dipolar strength in Fig. \ref{fig:s-a}. |
456 |
|
|
|
457 |
|
|
\begin{figure}[ht] |
458 |
|
|
\centering |
459 |
|
|
\caption{The amplitude $A$ of the ripples vs. dipole strength ($\mu$) |
460 |
|
|
for both the hexagonal lattice (circles) and non-hexagonal lattice |
461 |
|
|
(squares). In both simulations the dipole |
462 |
|
|
strength ($k_r$) was kept constant at a value of $1.987 \times |
463 |
|
|
10^{-4}$ kcal mol$^{-1}$ \AA$^{-2}$. The temperatures were also kept |
464 |
|
|
fixed at 230K for the hexagonal lattice and 260K for the non-hexagonal |
465 |
|
|
lattice (approximately 2/3 of the order-disorder transition |
466 |
|
|
temperature for each lattice).} |
467 |
|
|
\includegraphics[width=\linewidth]{picture/A-s.eps} |
468 |
|
|
\label{fig:s-a} |
469 |
|
|
\end{figure} |
470 |
|
|
|
471 |
|
|
\subsection{Non-hexagonal lattices} |
472 |
|
|
|
473 |
|
|
We have also investigated the effect of the lattice geometry by |
474 |
|
|
changing the ratio of lattice constants ($\gamma$) while keeping the |
475 |
|
|
average nearest-neighbor spacing constant. The antiferroelectric state |
476 |
|
|
is accessible for all $\gamma$ values we have used, although the |
477 |
|
|
distorted hexagonal lattices prefer a particular director axis due to |
478 |
|
|
the anisotropy of the lattice. |
479 |
|
|
|
480 |
|
|
Our observation of rippling behavior was not limited to the hexagonal |
481 |
|
|
lattices. In non-hexagonal lattices the antiferroelectric phase can |
482 |
|
|
develop nearly instantaneously in the Monte Carlo simulations, and |
483 |
|
|
these dipolar-ordered phases tend to be remarkably flat. Whenever |
484 |
|
|
rippling has been observed in these non-hexagonal lattices |
485 |
|
|
(e.g. $\gamma = 1.875$), we see relatively short ripple wavelengths |
486 |
|
|
(98 \AA) and amplitudes of 17 \AA. These ripples are weakly dependent |
487 |
|
|
on dipolar strength (see Fig. \ref{fig:s-a}), although below a dipolar |
488 |
|
|
strength of 5.5 Debye, the membrane loses dipolar ordering and |
489 |
|
|
displays only thermal undulations. |
490 |
|
|
|
491 |
|
|
The rippling in non-hexagonal lattices also shows a strong dependence |
492 |
|
|
on the internal surface tension ($k_r$). It is possible to make the |
493 |
|
|
ripples disappear by increasing the internal tension. The low-tension |
494 |
|
|
limit appears to result in somewhat smaller ripples than in the |
495 |
|
|
hexagonal lattice (see Fig. \ref{fig:kr-a}). |
496 |
|
|
|
497 |
|
|
The ripple phase does {\em not} appear at all values of $\gamma$. We |
498 |
|
|
have only observed non-thermal undulations in the range $1.625 < |
499 |
|
|
\gamma < 1.875$. Outside this range, the order-disorder transition in |
500 |
|
|
the dipoles remains, but the ordered dipolar phase has only thermal |
501 |
|
|
undulations. This is one of our strongest pieces of evidence that |
502 |
|
|
rippling is a symmetry-breaking phenomenon for hexagonal and |
503 |
|
|
nearly-hexagonal lattices. |
504 |
|
|
|
505 |
|
|
\subsection{Effects of System Size} |
506 |
|
|
To evaluate the effect of finite system size, we have performed a |
507 |
|
|
series of simulations on the hexagonal lattice at a temperature of 300K, |
508 |
|
|
which is just below the order-disorder transition temperature (340K). |
509 |
|
|
These conditions are in the dipole-ordered and rippled portion of the phase |
510 |
|
|
diagram. These are also the conditions that should be most susceptible to |
511 |
|
|
system size effects. The wavelength and amplitude of the observed |
512 |
|
|
ripples as a function of system size are shown in Fig. \ref{fig:systemsize}. |
513 |
|
|
|
514 |
|
|
\begin{figure}[ht] |
515 |
|
|
\centering |
516 |
|
|
\caption{The ripple wavelength (top) and amplitude (bottom) as a function of |
517 |
|
|
system size for a hexagonal lattice ($\gamma=1.732$) at 300K.} |
518 |
|
|
\includegraphics[width=\linewidth]{picture/SystemSize.eps} |
519 |
|
|
\label{fig:systemsize} |
520 |
|
|
\end{figure} |
521 |
|
|
|
522 |
|
|
There is substantial dependence on system size for small (less than 200 \AA) |
523 |
|
|
periodic boxes. Notably, there are resonances apparent in the ripple |
524 |
|
|
amplitudes at box lengths of 121 \AA and 206 \AA. For larger systems, |
525 |
|
|
the behavior of the ripples appears to have stabilized and is on a trend to |
526 |
|
|
slightly smaller amplitudes (and slightly longer wavelenghts) than were |
527 |
|
|
observed from the 240 \AA box sizes that were used for most of the calculations. |
528 |
|
|
|
529 |
|
|
It is interesting to note that system sizes which are multiples of the |
530 |
|
|
default ripple wavelength can enhance the amplitude of the observed ripples, |
531 |
|
|
but appears to have only a minor effect on the observed wavelength. It would, |
532 |
|
|
of course, be better to use system sizes that were many multiples of the ripple |
533 |
|
|
wavelength to be sure that the periodic box is not driving the phenomenon, but at |
534 |
|
|
the largest system size studied (485 \AA $\times$ 485 \AA), the number of |
535 |
|
|
molecules (5440) made long Monte Carlo simulations prohibitively expensive. |
536 |
|
|
We recognize this as a possible flaw of our model for bilayer rippling, but |
537 |
|
|
it is a flaw that will plague any molecular-scale computational model for |
538 |
|
|
this phenomenon. |
539 |
|
|
|
540 |
|
|
\section{Discussion} |
541 |
|
|
\label{sec:discussion} |
542 |
|
|
|
543 |
|
|
We have been able to show that a simple lattice model for membranes |
544 |
|
|
which contains only molecular packing (from the lattice), head-group |
545 |
|
|
anisotropy (in the form of electrostatic dipoles) and ``hydrophobic'' |
546 |
|
|
interactions (in the form of a nearest-neighbor harmonic potential) is |
547 |
|
|
capable of exhibiting stable long-wavelength non-thermal ripple |
548 |
|
|
structures. The best explanation for this behavior is that the |
549 |
|
|
ability of the molecules to translate out of the plane of the membrane |
550 |
|
|
is enough to break the symmetry of the hexagonal lattice and allow the |
551 |
|
|
enormous energetic benefit from the formation of a bulk |
552 |
|
|
antiferroelectric phase. Were the hydrophobic interactions absent |
553 |
|
|
from our model, it would be possible for the entire lattice to |
554 |
|
|
``tilt'' using $z$-translation. Tilting the lattice in this way would |
555 |
|
|
yield an effectively non-hexagonal lattice which would avoid dipolar |
556 |
|
|
frustration altogether. With the hydrophobic interactions, bulk tilt |
557 |
|
|
would cause a large strain, and the simplest way to release this |
558 |
|
|
strain is along line defects. Line defects will result in rippled or |
559 |
|
|
sawtooth patterns in the membrane, and allow small ``stripes'' of |
560 |
|
|
membrane to form antiferroelectric regions that are tilted relative to |
561 |
|
|
the averaged membrane normal. |
562 |
|
|
|
563 |
|
|
Although the dipole-dipole interaction is the major driving force for |
564 |
|
|
the long range orientational ordered state, the formation of the |
565 |
|
|
stable, smooth ripples is a result of the competition between the |
566 |
|
|
hydrophobic and dipole-dipole interactions. This statement is |
567 |
|
|
supported by the variations in both $\mu$ and $k_r$. Substantially |
568 |
|
|
weaker dipoles or stronger hydrophobic forces can both cause the |
569 |
|
|
ripple phase to disappear. |
570 |
|
|
|
571 |
|
|
Molecular packing also plays a role in the formation of the ripple |
572 |
|
|
phase. It would be surprising if strongly anisotropic head groups |
573 |
|
|
would be able to pack in hexagonal lattices without the underlying |
574 |
|
|
steric interactions between the rest of the molecular bodies. Since |
575 |
|
|
we only see rippled phases in the neighborhood of $\gamma=\sqrt{3}$, |
576 |
|
|
this implies that there is a role played by the lipid chains in the |
577 |
|
|
organization of the hexagonally ordered phases which support ripples. |
578 |
|
|
|
579 |
|
|
Our simple model would clearly be a closer approximation to reality if |
580 |
|
|
we allowed greater translational freedom to the dipoles and replaced |
581 |
|
|
the somewhat artificial lattice packing and the harmonic mimic of the |
582 |
|
|
hydrophobic interaction with more realistic molecular modelling |
583 |
|
|
potentials. What we have done is to present an extremely simple model |
584 |
|
|
which exhibits bulk non-thermal rippling, and our explanation of the |
585 |
|
|
rippling phenomenon will help us design more accurate molecular models |
586 |
|
|
for the rippling phenomenon. |
587 |
|
|
|
588 |
|
|
\clearpage |
589 |
|
|
|
590 |
|
|
\bibliography{ripple} |
591 |
|
|
|
592 |
|
|
\clearpage |
593 |
|
|
|
594 |
xsun |
2138 |
\end{document} |