Defects in Crystalline Packings of Twisted Filament Bundles: I. Continuum Theory of Disclinations
Abstract
We develop the theory of the coupling between inplane order and outofplane geometry in twisted, twodimensionally ordered filament bundles based on the nonlinear continuum elasticity theory of columnar materials. We show that twisted textures of filament backbones necessarily introduce stresses into the crosssectional packing of bundles and that these stresses are formally equivalent to the geometricallyinduced stresses generated in thin elastic sheets that are forced to adopt spherical curvature. As in the case of crystalline order on curved membranes, geometricallyinduced stresses couple elastically to the presence of topological defects in the inplane order. We derive the effective theory of multiple disclination defects in the cross section of bundle with a fixed twist and show that above a critical degree of twist, one or more 5fold disclinations is favored in the elastic energy ground state. We study the structure and energetics of multidisclination packings based on models of equilibrium and nonequilibrium crosssectional order.
pacs:
I Introduction
Topological defects are crucial components of the structure and thermodynamics in many frustrated systems in condensed matter (1). Perhaps the most wellknown example of frustrationinduced defects is exemplified by the Abrikosov phase of typeII superconductors where the application of a external magnetic field leads to the proliferation of vortices where the superconducting order is destroyed and through which magnetic flux is threaded (2). One remarkable feature of such frustrated systems is appearance of defects in the ground state, indicating that the balance of competing thermodynamic forces requires highly heterogeneous distributions of energy and structure. In geometrically frustrated systems, frustration arises intrinsically from the incompatibility of locallypreferred order with geometrical constraints on longrange ordering (3). Examples of geometrical frustration abound in selforganized molecular and colloidal systems. In bulk, threedimensional materials, well known examples include liquidcrystal blue phases (4) as well as the twistgrain boundary phases of chiral smectics (5). When confined to twodimensional surfaces, materials possessing a range of anisotropic order—nematic (6); (7); (8), hexatic (9), smectic (10); (11), crystalline (9); (12); (13); (14); (15); (16)—are generically frustrated by the presence of nonzero Gaussian curvature, which couples favorably to the presence of disclinations in the ground states.
Condensed phases of chiral polymers are subject to a unique frustration between twodimensional (2D) ordering perpendicular to the chain backbone and a microscopic tendency for intermolecular twist. Kamien and Nelson showed that in bulk columnar materials chirality gives rise to two distinct types of grainboundary phases—the tiltgrain boundary and moiré phases—both composed of arrays of dislocations lying in the plane of 2D order (17); (18). Underlying the frustration of bulk columnar phases of chiral polymers is the geometrical coupling between inplane displacements and filament tilts: interfilament twist requires gradients in inplane shear stresses along the molecular backbone. The frustration of chiral polymer assemblies is particularly important to the assembly of biological polymers, from extracellular proteins like collagen (19) and fibrin (20) to the cytoskeletal filaments, factin (21); (22). These are universally helical molecules and are organized into denselypacked states in cells and tissues of living organisms (23). A number of studies show that the frustration between 2D and chiral ordering gives rise to important thermodynamic properties including selflimiting assembly of bundles and fibers of chiral filaments (24); (25); (26); (27); (29); (28).
Recently, we have demonstrated that frustration between chiral order and 2D packing leads to another important and surprising consequence, the restructuring of the ground state packing of twisted filament bundles (30). In particular, we reported that twisted bundles are akin to 2D crystals formed on the sphericallycurved surfaces, in which outofplane geometry generates inplane stresses that are partially screened in the ground state by topological defects, 5fold disclinations, in the lattice order of bundle cross sections. Hence, it was proven that ground state inplane order of sufficiently twisted bundles is irregular, possessing an excess of topological defects in the configurations that minimize the elastic energy of filament packing.
In this article we describe in detail the theory of disclinations in twisted filament bundles and its derivation from nonlinear continuum elasticity theory of 2Dordered filament arrays. The unique symmetries exhibited by these materials lead to an intrinsic, nonlinear coupling between inplane strains and outofplane deflections of the filament backbone: interfilament twist makes it impossible to evenly space filaments in cross section. This analysis of the nonlinear theory shows that the equations of mechanical equilibrium in bundles are subject a compatibility condition linking twist of filament backbones and inplane stresses. In analogy to the Föpplvon Kárman theory of elastic plates and membranes, this compatibility condition for filament bundles shows that twist generates inplane stresses in bundles equivalent to those generated in a positivelycurved elastic sheet possessing a Gaussian curvature equal to , where is the helical pitch of the bundle. Motivated by the fact that topological defects screen curvatureinduced stresses in crystalline membranes, we derive the effective theory for disclinations in the cross section of twisted bundles. We show that above a critical of twist , 5fold disclinations are trapped in the cross section, where is the bundle radius. An example of a twisted bundle ground state possessing an energeticallyfavorable 5fold disclination is shown in Fig. 1. At higher values of twist, multiple disclinations are stabilized in the cross section of crystalline bundle packings. Based on the continuum theory, we study the discrete spectrum of elasticenergy minimizing configurations as a function of bundle twist which efficiently screen the buildup of twistinduced stresses. Further, we show that for a simple model surfacenucleated defects, the relatively weak repulsions between disclinations near the free boundaries of twisted bundles lead to a “pile up” of 5fold defects just above the critical size for disclination stability. The excess defects entrapped within these nonequilibrium structures suggest that a limited mobility of disclinations within the bulk of bundles drastically reduces the screening of geometricallyinduced stresses in “surfacegrown” bundles.
The remainder of this article is organized as follows. In Sec. II describe the rotationallyinvariant properties of the nonlinear elasticity theory of 2D ordered filament arrays (i.e. columnar order). In Sec. III we derive and study the equations of mechanical equilibrium for twisted bundles in the presence disclinations in the cross section, showing that one or more disclinations become stabilized by twistedinduced stress above a critical twist. In Sec. IV we present the results for multidisclination cross sections in twisted bundles for both groundstate packings and a model of nonequilibrium bundle assembly. We conclude with a brief discussion of the surprising correspondence between crystalline order on sphericallycurved surfaces and crystalline order of twisted bundles. Appendix A describes the coarsegraining of interfilament interactions and the form of the nonlinear elastic energy of multifilament assemblies. An important result of this study is the exact and closedform solution for the elastic energy of multiple disclinations in a 2D crystal, bounded by a free cylindrical surface. To our knowledge, no such solution has been previously published. As these results are more broadly applicable to finitesized crystalline materials beyond the specific context of twisted filament bundles we include the full details of the derivation of the disclinationinduced stresses and energies in Appendix B. In a subsequent paper (31), we analyze the role of dislocations—“neutral”, 57 pairs of disclinations—in groundstate order of twisted bundles as well as the structure and thermodynamics of multidislocation groundstates of twisted bundles.
Ii Rotational Invariance and the NonLinear Strain of Ordered Filament Arrays
In this section we construct the elastic energy that describes deformations of an ordered array of filamentous elements. We assume the stressfree reference state of this energy to be an equidistant hexagonal array of uniformly straight filaments, aligned along the direction. To describe deformations, we consider the mapping of a material point filament array in its reference configuration, , to the position of the same point in the deformed configuration, , where denotes the inplane components . We the define the inplane displacement , which the displacement of a point which, after deformation, is in a plane at . Here, it is most convenient to adopt a “mixed representation” where we define as function of material coordinates, , in the plane (a Lagrangian variable) and a function “current” vertical position, (a Eulerian variable) (32).
As filamentous assemblies possess a type of twodimensional order, it is essential to construct the strain in terms of a twodimensional strain tensor that describes changes in interfilament spacing in a plane perpendicular to the backbone orientation or chain tangent, . The tangent is related to the displacement by (33). This property is necessary to ensure that deformations that slide filaments along their long axis cost no mechanical energy. The elastic energy of a material with this type of columnar order (34) has the following form
(1) 
where is the elastic strain tensor which has components in the and direction only. Here, and are the Lamé elastic coefficients characterizing the inplane, isotropic elastic properties of the hexagonal filament lattice. The precise form of the strain tensor must be such that uniform rigid rotations of the reference state of the filament array require no elastic energy. The form of the strain satisfying these conditions is,
(2) 
In addition to the standard symmetric derivatives in the linear elastic strain, includes two nonlinear contributions which ensure rotational invariance of the strain. The combination of the first 3 terms in eq. (2), familiar to the nonlinear strain of 2D solids, is invariant under rotations around the axis (37). The the final term is necessary to preserve rotational invariance under rotations around an axis in the plane (33). It is straightforward to show, for example, that a rigid rotation around the axis by an angle by described by, leads to vanishing strain.
This final nonlinear contribution to the strain in eq. (2) from the outofplane derivatives of derives from the layered geometry of the filament array. The filament array can be decomposed into a series of rows, ruled surfaces, stacked along directions in the plane perpendicular to the filament tangent. And not unlike the nonlinear strain of fluid membrane stacks (i.e. smectics) (35), the elastic energy is insensitive to sliding these rows along the tangent direction, and hence, the nonlinear form of the strain ensures that the elastic energy measures distances perpendicular to . That is, if neighbor filaments are separated by in the plane, the nonlinear strain is sensitive to the perpendicular projection of this distance, or
(3) 
which measures the distance of closest approach between the filament pair. In Appendix A, for microscopic model in which filaments are treated as continuous curves whose segments interact via a central force law (such as a LennardJones potential) we show that the potential energy of the system is most naturally expressed as function of alone. Furthermore, by explicitly constructing distortions of this microscopic model from its mechanicallystable, hexagonallyordered reference state, we find that the coursegrained energy is identical to eq. (1) described by the nonlinear elastic strain tensor, , of the form eq. (2). Thus, the contribution from to the form of the nonlinear strain may be viewed as the result of the projection of interfilament distance changes in a plane perpendicular to , i .e. .
For the case of small strains, it is often sufficient to maintain the linearized strain tensor, . However, as materials with columnar order are particular “soft” to tilt or bend deformations due to the lack of outofplane shear response, inplane tilt deformations become significant in many situations. It has been demonstrated that the anharmonic coupling between inplane strains and filament tilt gives rise to outofplane buckling instabilities in columnar systems (33); (36). In particular, when subject to a sufficiently large uniform, uniaxial stress in the cross section of the material, the columns become unstable to certain longwavelength modes along the long axes of the cylinder, which reduce interfilament spacing at the expense of outofplane bending. Hence, these filamentous and columnar materials are subject to the same HelfrichHurault instability well known in smectic layer systems (40). In the following, we show that this instability, is a particular example of a more general phenomena in which stress in the plane of filament order couples to outofplane deformations of flexible filament arrays. Due to the generic form of the nonlinear coupling between filament tilt and elastic strain, we find that certain configurations of necessarily introduce stress into the array, in a way that is formally quite similar to the relationship between inplane stress and the Gaussian curvature of thin elastic sheets. For the purposes of the present study, we focus on the case of superhelically twisted bundles for which we demonstrate that the elastic energy ground state is, in general, highly complex and riddled with energyminimizing configurations of topological defects in the lattice order of the bundle cross section.
While it is important to keep in mind that is necessary to retain the contribution from to the strain for large inplane rotations that necessarily occur between distant planar cross sections of the twisted array, in the following we will drop the contribution from when referring to . Further, we use the fact that to write the nonlinear strain more simply as
(4) 
highlighting the geometrical coupling between inplane strains and outofplane geometry unique to the nonlinear theory of columnar materials.
Iii Mechanical Equilibrium in Twisted Bundles
In this section we derive the equations governing the mechanical equilibria of filament bundles that are superhelically twisted. Our primary task is to demonstrate that a necessary consequence of this apparently simple geometry is a nonuniform distribution of the stress in the cross section of the bundle. Hence, the appearance of stress in these bundles is an indication of the fact that it is geometrically impossibly to maintain a uniform spacing of filaments in the presence of twist (41). Our formulation of the twistinduced stresses in bundles casts this geometric frustration in a surprising light. From the point of the view of the stress distribution, global twist of the bundle acts like uniform distribution of disclinations in the cross section whose density increases with the square of the bundle rotation rate. Thus, our second task in this section is to demonstrate the energetic coupling between the presence of twistinduced stress and topological defects in the lattice order of the filaments.
iii.1 Equations of mechanical equilibrium
We consider a cylindrical bundle subject to a uniform rate, , of twist around the central axis of the bundle. Additionally, we assume that the cross sections of the bundle are identical up to a rotation. In this case, we decompose the displacements into two steps: 1) , the inplane displacement field from hexagonal order of a given reference plane of the bundle, say ; and 2) , the overall composite displacement resulting from helical rotation of positions at a constant rate, , around along the bundle.
(5) 
from which we find the inplane projection of the filament tangent configuration,
(6) 
This expression for —given in terms the current position, , of the filament in cylindrical coordinates—describes a socalled “doubletwist” texture, wellstudied in the context of liquidcrystal blue phases (4). Here, filament orientation rotates around the radial direction from the orientation, , at the bundle center to a maximum tiltangle,
(7) 
at the outer boundary, where is the cylindrical radius of the bundle.
In this paper, we consider the rate of bundle twist, , to be quenched, say by the presence of strong, chiral interfilament torques (27) or, instead, by some external mechanical force. According to helical symmetry described by eq. (5), the filament positions, displacements and strains are described by the state of a given plane at , with the bundle at other described by uniform rotations of these configurations around the central axis. In this case, the problem reduces to solving for in the twodimensional plane that minimizes the energy per unit length described by eq. (1), . Given the composite displacement field of eq. (5), the variation of the elastic energy with respect to components of gives
(8) 
where the stress tensor is simply
(9) 
The nonlinear coupling between inplane strain and outofplane filament tilt accounts for second contribution to the righthand side of eq. (8). This represents a mechanical coupling of inplane stress between different vertical layers of the bundle, which is absent from the linear theory of columnar order.
Below we show that twist gives rise inplane stresses, , or order . It is straightforward to show from eqs. (5) and (6) that the factor of inplane tilt, and derivative of contribute to each an additional factor of relative to the terms in (8). Hence, for the case that small twist, we approximate the EulerLagrange equations, , by the order terms and neglect the higherorder corrections deriving from interplane coupling which contribute at order . Based on this approximation, we arrive at the condition for mechanical equilibrium from the elasticity theory of isotropic materials, namely,
(10) 
along with the condition of vanishing normal stress at the boundary,
(11) 
The problem of mechanical equilibrium in twisted bundles is one of 2D elasticity for which it is most convenient to solve in terms of an Airy stress function (37), , related to the stress by,
(12) 
By construction, the stress derived from any function is divergencefree, satisfying mechanical equilibrium according to eq. (10). However, not every corresponds to a physical configuration, which requires the existence of a displacement field . That is, the solution for must be compatible with the definition of strain, .
Similar to the wellknown Föpplvon Kármán theory of thin sheets (37), we derive the compatibility condition for the Airy stress from the constitutive relationship between stress and strain,
(13) 
We cast the conditions that eq. (13) can be solved to find a displacement field by taking the antisymmetric derivatives of strain, , yielding the following compatibility relation for the Airy stress
(14) 
where we have used the definition of stain in eq. (4) and , is the 2D Young’s modulus of the array. For singlevalued strain functions, the first term on the righthand side must vanish, but in the presence of topological defects in the cross section, these terms generate nonvanishing sources for Airy stress.
In general, two types of topological defects contribute to the Airy stress of the twodimensional array: disclinations, associated with singular configurations of the bondangle field that points to the sixfold directions of lattice order; and dislocations, associated with singular configurations of that lead to no farfield rotation of the lattice directions (1). The bondangle field describes local rotations of the lattice directions in the cross section, and hence, is related to the antisymmetric, inplane derivatives of the displacement,
(15) 
In a hexagonal lattice, a disclination indicates a point around which increases or decreases by an integer multiple of ,
(16) 
where is the topological charge of the disclination. From Stokes theorem we have the the areal density of disclinations, ,
(17) 
where the sum over indicates a sum over multiple disclinations in the cross section. Likewise, a dislocation is defined in terms of a closed loop integral around which changes by an integer multiple of the lattice spacing, , along one of the sixfold directions,
(18) 
where is the Burger’s vector. The areal density of dislocations, , is therefore,
(19) 
By manipulating the displacement derivatives in the compatibility relation it is straightforward to show (12) that disclinations and dislocations generate pointlike and dipolelike sources, respectively for Airy stress,
(20) 
For the purposes of the present study, we focus on the case of disclinations only, , and solve exactly for the elastic energy of twisted bundles in the presence of arbitrary disclination configurations. In a subsequent study (31), we take advantage of the fact that more complex topological defects, dislocations and grain boundaries, may be constructed from neutral configurations of multiple disclinations, whose elastic stresses, according to the compatibility relation, are superposable.
In addition to the defectinduced sources for Airy stress, eq. (14) shows that certain gradients of inplane filament tilt generate a more homogenous source for due to the nonlinear coupling of tilt and strain. We denote these terms as the intrinsic twist, , of the bundle, which can written as,
(21)  
Indeed, by combining the disclination and tiltinduced sources for Airy stress we arrive at the final form of compatibility relation for ,
(22) 
When somewhere in the cross section of the bundle, eq. (22) tells us that there must be inplane stress.
Though is an unfamiliar geometric quantity, written in the form of eq. (21), we see that it is a total derivative of gradients of in the plane reminiscent of the socalled “saddlesplay” of a vector field, ,
(23) 
a total derivative term in the Frank elastic energy of nematicallyordered materials (34). The saddlesplay operator is most familiar when is the normal to a surface that is weaklydeflected from the plane, say a membrane, in which case, is the Gaussian curvature of the surface (42). From this point of view, the intrinsic twist, , plays precisely the role played by Gaussian curvature in the nonlinear theory of thin elastic membranes. In membranes, the inplane strain, , couples to outofplane deflections (12), described by the height function, , according to
(24) 
where the in the subscript is used to distinguish the nonlinear strain of membranes from the nonlinear strain of filament arrays, eq. (4). The compatibility relation for the inplane stress of membranes is known as the one of two Föpplvon Kármán relations, describing the mechanical equilibrium of thin plates (37). This relation was generalized by Seung and Nelson (12) to include the presence of topological defects in the crystalline order of membrane and is identical to eq. (22), with replaced by the Gaussian curvature of the sheet, calculated from eq. (23) and .
The compatibility equation for inplane stress encodes two fundamental properties unique to the nonlinear theory of membranes. First, it quantifies the inplane stretching needed to deform intrinsically flat sheets into shapes corresponding to , in accordance with the renowned Theorema Egregium of Gauss (42). And second, it demonstrates the formal equivalence between the farfield inplane stress distribution generated by localized regions of nonzero Gaussian curvature, and pointlike, orientational defects in the crystalline order of membrane, 5 or 7fold disclinations. Due to this second property, unlike crystalline order on planar 2D surfaces, topological defects—disclinations in particular—are well known to be necessary in the groundstates of crystalline order on surfaces with nonzero curvature, as disclinations of the appropriate charge are able to screen the curvatureinduced stresses inplane. An example of this frustration, important in structural studies of such diverse materials as fullerenes (43), viruses (44) and particlestabilized emulsions (15), is known alternately as the Thomson problem, which seeks to describe the lowestenergy arrangement of repulsive, pointlike particles on the surface of a sphere (45).
Though ordered filament bundles possess a unique geometry among 2D ordered materials, the mechanical frustration between inplane stresses and outofplane geometry in these materials is remarkably similar to that predicted by the nonlinear elastic theory of membranes. In the case of filament bundles, the intrinsic twist plays the role play by Gaussian curvature in membranes, necessarily introducing distortions of the interfilament spacing. Given the striking similarity, it is tempting, perhaps, to identify with the Gaussian curvature of some surface or set of surfaces, say, to which filaments are normal. Such an identification easily fails for any twisted configuration of filaments , for which no such surfaces exist (46), and yet is demonstrably nonzero. For the case of superhelical twist considered here, we find,
(25) 
Thus, superhelical doubletwist generates a homogeneous and negative source of Airy stress in the cross section. In this sense, we find that the inplane stresses induced by bundle twist are formally equivalent to those induced by positive Gaussian curvature in thin sheets. Formally, we may think of the intrinsic twist, , as a uniform density of negatively charged disclinations, continuously distributed throughout the bundle cross section. Hence, as the bundle grows larger in radius, the integrated topological charge of this distribution grows as , demonstrating that the frustration between uniform filament spacing and bundle twist grows rapidly with bundle size.
Finally, though twist generates stresses that are formally equivalent to those in sphericallycurved membranes, it is important to point out a key difference between the optimal packing of twisted bundles and the Thomson problem. Due to their closed topology, the bond network of point packings covering the sphere are required to possess exactly 12 excess 5fold disclinations in all configurations, a requirement of topology rather than a groundstate property (13). Due to the presence of a free boundary, the problem of a twisted, 2Dordered filament bundle is more closely aligned with the problem of a finitesized crystalline domain on a sphericallycurved surface (47). The presence of a free boundary in of twisted bundle or curved crystal allows the net number of disclinations (5 or 7fold) to adjust according the energetic balance of disclinations needed to screen geometricallyinduced stresses. Furthermore, as we show below, the requirement that normal components of stress vanish at the boundary of the domain leads to a strongposition dependence of the energetic costs for disclinations in various positions in the bundle cross section.
iii.2 Elastic energy of disclinations in twisted bundles
In this section we present the exact solution for the Airy stress of twisted, cylindrical bundles with multiple disclinations in the cross section, and derive the effective elastic energy depending only on and the positions and topological charges of disclinations. We seek a solution to the compatibility relation,
(26) 
The elastic energies of sufficiently twisted bundles show a clear preference for an excess of 5fold disclinations, indicating that the groundstate packing of twisted bundles is complex and irregular.
This basic result is clearly demonstrated by considering the stress of a twisted bundle possessing a single, centered disclination. Denoting as the stress induced by intrinsic twist,
(27) 
we search for the form which satisfies stressfree boundary conditions. In polar coordinates the components of stress are related to by,
(28) 
(29) 
and
(30) 
Hence, for the case where is axisymmetric, the conditions that at the boundary reduce to . The solution to eq. (27) subject to this boundary condition is
(31) 
A single disclination at generates a stress denoted by , satisfying,
(32) 
and the stresscondition at . The solution for for a centered disclination in a 2D circular cross section is known from ref. (12),
(33) 
From the Airy stress functions we have the twist and disclinationinduced pressure fields,
(34) 
and
(35) 
Notice that the intrinsic twist induces as a dilation at the core of the bundle, for , and compression at the periphery, for . This trend is reversed for a positively charged disclination, such as a 5fold defect, where for and for . Hence, the induced stresses of 5fold disclinations have a tendency to neutralize, or screen, the twistinduced stresses that derive from the nonlinear coupling between inplane strain and filament tilt.
As a result of this tendency, the elastic energy associated with bundle twist and disclinations are strongly coupled. From the Airy stress, the elastic energy can be computed from , which using eqs. (9) and (13), can be manipulated to yield
(36) 
The second term in the integrand above is equivalent to the total derivative, , whose contribution, therefore, vanishes due to the stressfree boundary condition. Hence, the elastic energy derives directly from the inplane pressure distribution, ,
(37) 
The first term above represents the unscreened, nonlinear elastic cost of bundle twist, whose  and dependence derives from the twistinduced strain, . The second term represents the selfenergy of a single disclination, which can be understood in terms of the constant axial strain required to remove or add angular wedges to the lattice, . The final term in eq. (37) represents the interaction between twist and disclinations. The sign of this term indicates a favorable interaction between twist and 5fold disclinations, , due to mutually screening of the farfield stresses generated by these distortions. However, while the elastic cost of twist depends continuously on , disclination charge is discretized in units of . The minimal topological charge of 5fold dislocations sets a critical value of bundle twist,
(38) 
above which the elastic screening by the disclination is sufficient to compensate for the defect selfenergy cost. According continuum theory, bundles twisted beyond this threshold are unstable to the incorporation of one or more 5fold disclinations in the cross section of the filament lattice.
The calculation of the elastic energy of multidisclination configurations follows a similar method to the case of a single, centered disclination. However, when one or more defects is offcenter, the stress is no longer axisymmetric, requiring a somewhat more complex form. Though algebraically tedious, the solution to eq. (22) proceeds by a standard multipole expansion of the disclinationinduced stresses. Ultimately, the infinite series representing defect interactions with twistinduced stress as well as defectdefect interactions for disclinations in arbitrary positions can be resummed exactly to yield the relative compact expressions in the effective theory for defects in twisted bundles described below. As we know of no other published calculation of the exact disclination energy in cylindrical and circular crystals, we present the full details of this analysis in Appendix B. We note that this theory may have other applications, for example, for multidisclination configurations in curved domains of 2D crystalline membranes. In the remainder of this section, we outline the solution and summarize the results.
Consider a disclination at polar coordinates in the cross section of the bundle. Following ref. (48) we decompose the Airy stress of the defect into a direct term, , describing the singular stress at the core, and an induced term, , due to the interaction of the defect with the free boundary. In the presence of a disclination of charge, , the direct stress at a point in the cross section has the form
(39) 
where, and . To determine the form of the induced stress, we consider the multipole expansion of ,
(40) 
The induced stress satisfies, for and has the generic form
(41) 
with . The coefficients and are determined by boundary condition, at . In terms of the Airy stress, the radial stress components vanish at the boundary when (48)
(42) 
and
(43) 
With the coefficients determined (see Appendix B), we evaluate the stress induced by the free boundary from,
and from eq. (89) we have the total pressure distribution of the disclination,
(44) 
where , and measures the square distance to an “image” defect of opposite charge outside of the bundle representing the screening of the elastic stress by the free boundary.
As shown in Appendix B, the stress profile of multiple disclinations may be superposed along with the twistinduced stress, , and the total elastic energy may be calculated by area integration of , yielding the effective energy quoted in ref. (30), which may be decomposed into 3 parts,
(45) 
Here, is the nonlinear elastic cost of bundle twist derived in eq. (37). From eqs. (105) and (106) we may combine the selfenergy and twistdisclination interaction into a single disclination energy, ,
(46) 
described in terms an effective, positiondependent potential for disclinations in twisted bundles,
(47) 
Finally, the interactions between disclinations are described by
(48) 
where
(49) 
It is straightforward to check from eqs. (47) and (49) that both the elastic selfenergy and the disclination interactions vanish when , a signature of the stress free boundary condition.
The key result of this analysis is the mutual screening of the elastic stresses of twist and disclinations in the bundle cross section described by the effective, single disclination potential . Both the selfenergy disclinations and the elastic interactions between twist and disclinations—respectively, the terms proportional to and in eq. (47)—are strongest for disclinations at the core of the bundle and decrease to zero as disclinations are pushed to the boundary of the bundle. However, while the selfenergy always prefers to expel disclinations to the boundary, for the interaction between disclinations and twist can either be attractive or repulsive, depending on the sign of . As discussed above, 5fold disclinations, with positive topological charge (), are attracted by the twistinduced stresses to the core of the bundle. For small twist, , the selfenergy of defects dominates over the elastic screening of twist, and is repulsive, with a maximum for disclinations at the core, . However, for sufficiently twisted bundles, , the net elastic energy of single disclinations is attractive, favoring 5fold disclinations at the core the bundle. This attractive regime indicates that the screening of twistinduced stress dominates the elastic selfenergy of defects, and ultimately, suggests that the optimal, groundstate packing of filament bundles of fixed twist are irregular, including one or more topological defects in the cross section.
Before analyzing the structure of these multidisclination groundstates in the next section, we briefly discuss the global stability of 5fold disclinations in bundles that are free to relax both the radial position of the defect, as well as the bundle twist. Fig. 2 shows a contour plot of the elastic energy, , of a bundle possessing a single 5fold disclination as a function of radial position, , and bundle twist, . In the absence of an external source for twist (i.e. imposed torque) or intrinsic source for twist (i.e. chiral filament interactions), the global minimum occurs when disclinations are expelled from untwisted bundles, . Fig. 2 shows three additional critical points for and , where both the radial force on the disclination, , and the twistmoment on the bundle, , vanish. The point is a local maximum describing the selfenergy of a centereddisclination in an untwisted bundle, . Despite the absence an explicit energetic preference for bundle twist, we find that there exists a metastable twisted state for and , with a 5fold disclination trapped at the bundle center for which , the elastic cost of incorporating a disclination is significantly reduced due to the screening disclination stress by twist. Finally, there is an unstable saddlepoint separating the 2 minima at and , for which .
The lateral motion of a disclination in 2D crystals requires a global repositioning of all lattice sites in the cross section, and therefore, we should expect the relaxation kinetics associated with defects under the forces described by to be extremely slow. Here we show that even in the absence of kinetic limitations on disclination motion, the nonlinear elastic energy of filament bundles provides a thermodynamic mechanism to trap 5fold disclinations in the cross section. Assuming a crude model of overdamped kinetics of bundle twist, , and defect motion, , where and are damping coefficients, we expect weakly twisted bundles to expel disclinations that originate outside of the bundle core as the system evolves to a lower energy. However, when disclinations originate deep within the interior, the state of the bundle develops a finite twist, , and the disclination is entrapped within the bundle center. The boundary separating these two dynamical behaviors is shown as dashed line in Fig. 2. While the entrapped disclination is ultimately thermodynamically unstable to expulsion from an untwisted bundle, there is an appreciable activation energy, , proportional to the bundle volume, which must be overcome in order to remove the defect from the core of the twisted bundle. For this reason, we argue that despite the extensive elastic energy needed to form them, due to the elastic screening provided by twist 5fold disclinations formed at the core of twodimensionally ordered filament bundles are especially longlived, if not, permanent structural defects even in achiral materials, for which their is no intrinsic preference for bundle twist.
Iv MultiDisclination Cross Sections of Twisted Bundles
In this section we analyze the elasticenergy ground states of twistedfilament bundles based on the continuum theory of topological defects derived in Appendix B and summarized in eqs. (45)  (49). These equations account only for the longrange elastic costs of deforming the array, and do not account, specifically, for the shortlength scale effects captured by the core energy of disclinations, . In the following, however, we neglect this finite energy contributions in comparison to the elastic selfenergy of disclinations that scales with , and hence dominates in the limiting case of large bundles.
iv.1 Equilibrium packings of twisted bundles
In this section, we consider the minimalenergy configurations constructed from an integer number of 5fold, , disclinations. According to the singledisclination elastic energy, eq. (47), for 5fold disclinations are attracted to the core of a twisted bundle. While the nonlinear stresses generated by twist attract disclinations to the bundle core, disclinations of equal sign repel one another at long range, countering the tendency to entrap an arbitrarily large number of defects in the core.
Determining the ground state of disclinations in twisted bundles is, thus, not unlike the classical groundstate of longrange repulsive particles confined to finite, twodimensional clusters (49); (50); (51). Such problems arise in a range of physical contexts including the Wignercrystal states of electrons in mesoscopic particles (53), 2Dconfined colloidal crystals (52) and multivortex states of superconducting discs (54) and quantum dots (55). The models previously studied differ from the present specifically in terms of the nature of both repulsive interactions and the effective confining potential. Unlike the very longrange elastic interactions between disclinations described by eq. (49), the longrange potentials studied in previous cases are typically inverse power law for or logarithmic functions of separation. Additionally, the elastic screening by the stressfree boundary in the present model leads to disclination interactions, eq. (49), that are weakened as either disclination approaches the boundary.
The groundstate configurations of twisted bundles with only 5fold disclinations were determined for twists in the range of by direct comparison of the energies of defect configurations consisting of one or two disclination “shells”, a geometry common to fewparticle groundstates of repulsive 2D clusters (49). Each shell is composed of a symmetric arrangement of disclinations. For a given twist, the elastic energy of the bundle cross section is minimized over the radii of the inner and outer shells, as well as the angular correlation between the shells. The energy, structure and total disclination number of groundstate configurations are shown in Fig. 3. For bundle twist in the range , the ground states possess a single shell of disclinations, while for higher twists, a second radial shell of disclinations is favored.
While twist and its associated inplane stresses increases continuously, the number of disclinations in the groundstate is quantized. Figure 3b shows the stepwise increase in disclination number in increasingly twisted bundles, a roughly linear function of . The slope of the increase in disclination number is consistent, approximately, with the number of 5fold disclinations required to “neutralize” the effective topological charge of defect and twistinduced stresses. From eq. (22), we see that outofplane twist leads to an effective topological disclination charge per unit area, . For a bundle of radius, , the number of disclinations needed to neutralize this background charge can be estimated as,
(50) 
which is plotted as dashed line in Fig. 3b for comparison to optimal disclination structures. While the slope of this curve is roughly consistent with the defect number found by minimization of multidisclination energy, notice that the number of disclinations predicted in the ground state is consistently less than , suggesting that the neutrality condition is not precisely maintained for small bundles where much of twistinduced stresses are screened by the stressfree boundary condition.
For large bundles, we expect the ground state predicted by the continuum theory of eq. (LABEL:eq:_Etoto) to converge asymptotically a neutral, “Wigner lattice” of disclinations. The elastic energy of this configuration of the Wigner lattice can by calculated from the periodic solution to eq. (22) for the inplane pressure for an infinite plane,
(51) 
where are the reciprocal lattice vectors of a 2D lattice of areal density (56). Assuming the ground state of the Wigner lattice is a hexagonal array of disclinations, we calculate the elastic energy in the limit from the lattice sum,
(52) 
Here, where , the Wignerlattice spacing of disclinations. This constant value is shown as a dashed, horizontal line in Fig. 3a. As indicated by the series of multidisclination groundstates found for , the appearance of 5fold disclinations in the cross section of twisted bundles accounts for a crossover from a increase of the energy density to the ultimately twistindependent value of the infiniteradius, Wigner lattice state.
It must be noted that in the forgoing analysis and derivation of the effect disclination energies, in the equations of mechanical equilibrium, eq. (10), we have neglected terms that are higherorder in that derive from coupling of stresses in different vertical layers of the bundle. Clearly, the inclusion of these effects must have a significant impact on the structure and energy of multidisclination ground states for large values of reduced twist, when . However, the predicted value of where the bundle becomes unstable to a single disclination, as well as the transition to multidisclination ground states, fall well within the regime of twist where we expect the corrections to the approximate theory to be modest.
iv.2 Nonequilibrium disclination arrays in surfaceassembled bundles
The motion of disclination lines in twisted bundles of filaments is slow, and in many realistic scenarios the positions of disclinations that form in the cross section of twisted bundles are likely to be quenched during the assembly process. The displacement of a disclination, say by a distance of one lattice spacing in the cross section, requires the absorption or emission of a dislocation, a neutral disclination pair, which in turn must diffuse from the disclination to the free boundary of the crystal (57); (58). Hence, the motion of a disclination over a distance of order , requires a sequence of roughly dislocations to glide a distance of order lattice spacings. We may crudely estimate the timescale for disclination motions within a 2D crystal grow at least as quickly , where the factor of bundle length accounts for the fact that disclinations run along the full length the bundle. All of this suggests that over the times scales during which the selfassembly process occurs, it is quite reasonable to expect that disclination motion is negligible, and therefore, the most probable state of even highlytwisted filaments assemblies will be markedly different from the equilibrium, multidisclination states discussed in the previous section.
In this section we explore a simple model for the nonequilibrium formation of twistedfilament bundles in which the topological reorganization of the cross section is inhibited by the sluggish dynamics of disclinations. In this model we assume that disclinations can only form at the free surface of a bundle as new filaments adhere to a partiallyformed bundle. Upon nucleation of disclinations within a surface layer of newlyadsorbed filaments, defects are then assumed to be frozen in position as further layers of absorbed filaments are assembled on the bundle.
To study the cross sectional order within this model of surface assembly we construct the following algorithm where concentric radial layers of filaments are absorbed sequentially to a bundle of fixed rotation rate, .

Add radial filament layer of width to preexisting bundle, increasing outer filament tilt by an increment, .

Consider addition of new disclinations at radial position, , by minimizing eqs. (45) over new defect number and angular position. Additional disclinations are subject to repulsive interactions within incipient layer, as well as with defects trapped within bundle from earlier stage of growth.

Energetically favorable defects are trapped within growing bundle and maintain their inplane position upon growth of further surface layers.
The minimization over disclination number and angular position is carried out numerically, and at each step in the radialassembly process, the total number of disclinations, , and total energy of the twistedbundle cross section are determined.
In Figure 4 we show results for the surfaceassembly model of twisted bundles with 5fold disclinations in the cross section. These demonstrate that structures of the multidisclination cross sections are both very distinct from the equilibrium cross sections of Fig. 3, as well as crucially sensitive to the tilt per filament layer, . According to eq. (47), the stability of disclinations in twisted bundles is determined entirely by the reduced twist, , the critical value of which is , is the same for all interfilament spacings , allowing us to correlate the magnitude of the tilt increment with the size of a bundle at the critical twist. A smaller value of tilt per layer, , implies that the bundle will be larger when it reaches the critical twist for stable disclinations. This critical radius for disclinations is , in units of filament spacing.
Figure 4a shows the energy density of surfaceassembled bundles for four values of tilt increment: and . Surfaceassembled bundles share the same energydependence below the critical value of twist, and each show a characteristic maximum in due to the presence of 5fold disclinations at higher twist. Notably, these energies “overshoot” the groundstate energy density above the critical value of , and the extent of excess energy (relative to the groundstate) depends sensitively on tilt increment per layer, increasing dramatically as is diminished. In this model of assembly, larger bundles, measured in terms of , screen twistinduced stresses less effectively than smaller bundles by the incorporation of 5fold defects at their free boundaries. This effect can be traced to the number of disclinations which are captured in the first few radial layers of growth beyond the critical size.
The number of disclinations captured, , at different values of , is shown in Figure. 4b for the same four values of . Each assembly exhibits an immediate “pileup” of 5fold disclinations in the outer layers as soon as the bundle grows beyond the size necessary to stabilize a single disclination, . That is, just above the critical size, these assemblies jump from a defectfree state to assemblies with and disclinations, respectively, for and
In Figure 4 (c) we analyze the number of disclinations in the first radial “shell”, , as a function of . Here is identified from the initial plateau value of beyond the critical twist. Two trends are immediately apparent. First, the value of is oscillatory with respect to . Second, the mean number disclinations (the amplitude of the oscillatory envelope) in the first shell decreases with . The oscillations in are simply due to the commensurability of a finite number of layers, , of finite radial thickness, , with the critical bundle size, . The number of layers of radial growth achieved when the bundle has grown just beyond the critical size is simply . In the model of radial growth, a bundle will therefore be quenched just beyond the critical twist by an amount, , at the point when the first shell of disclinations forms. It can shown that due the integral nature of layer addition, this degree of overtwist oscillates with increasing over a range 0 and with a period roughly corresponding to .
The decrease of the mean value with can be related to the weakening of repulsive interactions of disclinations near to the free boundary of the bundle. According to the effective energy of disclinations in twisted bundles, eq. (45), defects added near to the bundle boundary at leads to an elastic energy gain of roughly, . Opposing the incorporation of multiple disclinations in the surface layer is the cost of interdisclination repulsions. From eq. (49), when defects approach the surface of the bundle such that (or ) the interdefect potential approaches zero as
(53) 
Assuming a multidisclination shell with defects spread evenly within a radial layer at , we estimate the total cost of disclination repulsions per shell as roughly . Although the favorable coupling between disclinations and twist vanishes as defects approach the bundle surface like , the strength of disclinationdisclination repulsion vanishes more rapidly as , and thus, provides a weak resistance to the pileup of disclinations at the surface layer of the bundle. Optimizing the net elastic energy gain over the number of disclinations in the first shell we expect,
(54) 
where the overtwist may be approximated by . This analysis shows, consistent with numerical results, that the number of disclinations in the first pileup layer diverges as .
The results of the simple kinetic model of bundle growth suggest that the efficiency of twist screening by elastically favorable 5fold disclinations in nonequilibrium bundles is highly dependent on tilt per radial layer, . Interactions between surface defects in bundles composed of relatively few filaments upon reaching the critical twist (i.e. is relatively small) tend stabilize the cross section against pileup of excess disclinations. While the excess defects trapped at the surface of relatively larger bundles ultimately lead to additional elastic costs to further bundle growth as the surface defects must ultimately be incorporated into the core of the bundle, where interdisclination repulsive costs are greatest.
V Discussion
In this article, we studied the influence of outofplane geometry on the inplane packing of twisted and twodimensionally ordered filament bundles based on nonlinear continuum elasticity theory. Formally, this influence derives from the unique form of the nonlinear 2D strain tensor describing deformation of columnar order, which couples interfilament strains and tilting of filament backbones. Analysis of the equations of mechanical equilibrium in filament bundles shows that helical twist generates stresses in the bundle cross section that are formally equivalent to those generated by positive (spherical) Gaussian curvature of the 2D elastic sheet. In analogy to the problem of the curved, crystalline membranes, we also find here that these geometricallyinduced stresses may be screened, in part, by 5fold disclinations defects in the cross section of the bundle.
We derived the effective theory of disclinations in the cross sections of twisted bundles and, based on this theory, studied the multidisclination states of bundles for fixed reduced twist, . In equilibrium structures, disclinations appear above a critical twist, , and unlike the energy of the defectfree bundle, which grows unbounded with , the energy of the disclinationpossessing groundstates remains below a finite, upper bound provided by the infinitetwist, Wigner lattice of disclinations. In a simple model of nonequilibrium assembly of the twisted bundles, we show that the strong screening of disclinationdisclination repulsions by the free boundary of the bundle leads to an instability to “pileup” excess disclinations at the surface of a bundle when the bundle grows to the critical value of reduced twist. As the number of defects in these nonequilibrium packings far exceeds the number needed to neutralize the geometricallyinduced stresses, in this model of bundle growth the presence of 5fold disclinations is much less effective at reducing the inplane elastic stresses that may act to limit the lateral growth of bundles during the assembly process.
Underlying complex structure of the crosssectional order in twisted bundles is the surprising and unusual connection highlighted by nonlinear elasticity theory between crystalline order on sphericallycurved surfaces and in twisted bundles. We note here that the results of two similar models of chiral and biaxiallyordered materials anticipate this connection. The first was demonstrated by Kamien for a chiral, liquidcrystal phase with both nematic and hexatic order, the socalled phase (59). Here, the sixfold bondorientational order is represented by a vector field, , in a plane normal to the local nematic director, . The geometric relationship between and —encoded in the MerminHo relation—leads to the impossibility of uniform hexatic order for certain textures of the nematic director. Indeed, for the doubletwisted texture studied here, the intrinsic geometry of the nematic frustrates inplane hexatic order in precisely the same way that curvature frustrates hexatic order formed on a spherical surfce. Hence, in large doubletwisted domains of the phase, just as in spherical hexatics, positively charged, 5fold disclinations are favorable to screen geometricallyinduced stresses.
Further evidence of the formal equivalence between frustrated order in twisted bundles and on spherical surfaces was demonstrated by Kléman in studies of ideal packings of twisted filaments in an intrinsically curved, threedimensional space, namely (60); (61). The results of these studies derive from the Hopf fibration, which decomposes into linked geodesic curves, great circles, that are each associated with a unique point on (3). The geometry of has the property that: 1) any two great circles are equidistant and twist helically along their length; and 2) the distance between them in is half of the separation of their associated points on . Hence, any equallyspaced arrangement of points on corresponds to a perfectlypacked (maximum density) and twisted configuration of curves, or filaments, in . In this case, the problem of point packings on has a onetoone mapping onto a twisted fiber packing of . It is less clear at present, however, how this mapping may be used to study twisted filament packings in Euclidean space, as no projection from to preserves curve separations, leading to a second level of frustration associated with the flattening out of ideal packings of in addition to the frustration of point packings on already encoded in the fibration. As with a certain other geometrically frustrated problems—notably liquid crystal blue phase textures and icosahedral order in amorphous materials (3)–exploring the structure and energetics of ideal, twisted filament packings of projected to may ultimately provide a useful alternative avenue for studying chiral filament packing from a fundamentally geometrical point of view
We conclude this article with a few remarks regarding the potential for observations of multidisclination ground states in filamentous systems known to form twisted bundles or fibers. According to continuum theory, in both equilibrium and nonequilibrium bundles the key parameter determining the appearance of 5fold disclinations is the reduced twist, , with a critical value . This corresponds to a maximum tilt angle of the outer most filament of with respect to the bundle axis. This high degree of bundle twist has been demonstrated in coarsegrained simulation models of filament assembly (62), and hence 5fold defects are readily observed in the cross sections of simulated assemblies of chiral filaments (28). However, this critical tilt exceeds the value observed for all if not most twisted, biofilament assemblies. The collagen fibers that are observed to twist helically reach a maximum tilt angle of (19). The pitch and radius distributions of fibrin fibers have been well characterized in vitro by Weisel et al. (24), showing a maximum radius of roughly 50 nm and a mean pitch 1.9 , corresponding to an outer filament tilt of approximately , falling well below the threshold at which disclinations become stable. It is notable, however, that under certain conditions fibrin fibers are observed to grow to much larger radii, at which point the inplane packing becomes highlydisrupted, leading to a significantly more diffuse, and possibly fractal, organization at the fiber periphery. In light of the present study, we speculate that the appearance of disrupted inplane packing of fibrin fibers beyond a critical size may be a remnant of the disclination pileup that is predicted to occur in the nonequilibrium assembly model.
Acknowledgements.
The author would like to thank A. Azadi and I. Bruss for their careful review of this manuscript, as well as T. Lubensky for helpful discussions. This work was supported by the NSF Career program under DMR Grant 0955760.Appendix A CoarseGrained Elastic Energy of a Microscopic Model of SelfAssembled Filament Bundles
In this appendix we analyze a microscopic model of filamentous assemblies and deduce the form of the elastic energy via a coarsegraining of the microscopic degrees of freedom. Our purpose is to demonstrate explicitly that the form of the elastic energy in eq. (1) described specifically in terms of the nonlinear strain of eq. (2) arises naturally for ordered filament bundles forming under the influence of generic and mutuallyadhesive interactions. For simplicity, we assume that interactions between a pair of filaments, labeled and , may be described by the following interaction energy,
(55) 
where (or ) denotes the integration over the arclength of the central backbone of filament (or ) which is described by (or ). Here, is the pair potential describing interactions between segments on different filaments, which we assume to be shortranged and to be a function of for simplicity. We carry out the second integration over for a fixed by identifying as the arcposition on at the same vertical height as . We may then approximate to second order in as,
(56) 
where , and are the tangent, normal and curvature of filament evaluated at . At each position we denote the inplane separation between the curves as , while the square separation between two points at different vertical positions is approximately given by,
(57) 
where we have suppressed the dependence for clarity. In densely packed array, we expect filaments to be sufficiently straight on the scale of interfilament separation so that and we may ignore the curvature correction to above. With this approximation, the separation between curves and obtains a minimum for arcseparation,
(58) 
which denotes the closest point to on , or the distance of closest approach,
(59) 
Hence, is perpendicular to at , and expanding around the distance of closest approach , we have the separation between points on and ,
(60) 
Inserting this into eq. (55) and integrating over we find that we may express the interaction between and as the integral over of a natural function of , the local distance of closest approach,