## Abstract

Controlling the self-assembly of supramolecular structures is vital for living cells, and a central challenge for engineering at the nano- and microscales^{1,2}. Nevertheless, even particles without optimized shapes can robustly form well-defined morphologies. This is the case in numerous medical conditions where normally soluble proteins aggregate into fibres^{3,4}. Beyond the diversity of molecular mechanisms involved^{5,6}, we propose that fibres generically arise from the aggregation of irregular particles with short-range interactions. Using a minimal model of ill-fitting, sticky particles, we demonstrate robust fibre formation for a variety of particle shapes and aggregation conditions. Geometrical frustration plays a crucial role in this process, and accounts for the range of parameters in which fibres form as well as for their metastable character.

## Main

Identical cubes can pack into dense space-filling aggregates, but most shapes do not. As a result, the aggregates formed by these shapes tend to be frustrated, giving rise to arrested, glassy states^{7,8}. In protein aggregates, this frustration can arise from, for example, deformed or partially denatured protein domains, the juxtaposition of residues with unfavourable interactions, or sterically hindered hydrogen bonding. The global morphology of compact packings of these objects thus involves a competition between geometrical constraints, which hinder the formation of compact aggregates, and the particles’ overall attractive interactions.

To explore this competition in its simplest form, we consider two-dimensional, deformable polygons driven to aggregate by zero-range attractive interactions (Fig. 1a, b). We parametrize the magnitude of this attraction by a surface tension whose value controls the aggregate morphology (Fig. 1c). A low surface tension thus favours thin tree-like aggregates composed of undeformed particles with very little elastic frustration, reminiscent of so-called empty liquids^{9}. Conversely, a large surface tension leads to space-filling aggregates in which all particles are substantially deformed. In this paper, we demonstrate that fibres form at intermediate values of the tension, where the characteristic energies associated with particle attraction and deformation are comparable. We quantitatively account for these values based on the role of frustration, and show that fibres are very robust to changes in microscopic parameters, aggregation protocol and seeding conditions. Finally, we show that, despite this robustness, fibres do not constitute the ground state of our aggregates. Instead, they are kinetically trapped metastable states, consistent with their inherent frustration and with the well-documented irreversible character of protein fibre assembly *in vivo*.

We consider *n*-sided polygons, and use a deformation energy *e*^{(α)} for the *α*th polygon that is a function of its area *A*^{(α)} and of the lengths {*ℓ*_{i}^{(α)}}_{i=1…n} of its sides (Fig. 2a). In the following we use both regular and irregular polygons (as in Fig. 1b), and characterize the latter by an asymmetry parameter *k* ≥ 1, where *k* → 1 is the regular polygon limit while *k* → + *∞* yields short sides with vanishing rest length (see Methods). Minimizing the energy *e*^{(α)} with respect to the positions of the polygon’s vertices yields a rigid elastic ground state of energy *e*_{g} (Fig. 2b). Aggregates are formed by connecting multiple polygons through the joining of one or several of their sides. Two joined sides are treated as a single object, implying that they share the same two end-vertices (Fig. 2a). Side joining is favoured by the adhesion energy between particles, modelled by an energy penalty *σ* > 0 for each unjoined side regardless of its actual length. Thus, *σ* parametrizes the surface tension introduced in Fig. 1c. However, side joining also involves a distortion of the mismatched polygons, and thus increases their deformation energy above *e*_{g}.

A tree such as the one of Fig. 1c is always in its elastic ground state. Its average energy per particle is entirely due to surface tension, and reads *e* ∼ (*n* − 2)*σ* in the large-system limit (see Methods). A large bulk, on the other hand, has a negligible surface energy but a finite deformation energy *e* ∼ *e*_{b} − *e*_{g}, where *e*_{b} denotes the minimal deformation energy for a polygon constrained by the bulk topology (Fig. 2c). Rescaling the elastic energy and tension through and , we obtain for a tree and for a bulk. These rescaled energies make it clear that adhesion overcomes frustration, and trees become less stable than bulks at high tensions, with a transition at . As a result, if fibres indeed form as a result of the competition between these two effects, we expect them to appear for a dimensionless tension of order one.

To test this hypothesis, we simulate irreversible aggregation starting from a single polygon. Our algorithm mimics irreversible protein aggregation, where a particle binding to an existing aggregate does so in the most energetically favourable location without substantial rearrangements of the pre-existing aggregate topology. Throughout this process the aggregate energy is always minimized with respect to all vertex positions, imposing force balance before the aggregate energy is assessed (see Methods). We first grow aggregates of 150 irregular hexagons. The unfrustrated *k* = 1 case simply yields the bulk of Fig. 1a up to very large values of *σ*. Next, considering substantially frustrated hexagons with *k* = 2, we observe bulks at high tensions (), while low tensions () yield irregular tree-like aggregates (Fig. 3a). By contrast, periodic fibres form at intermediate tensions, and maintain perfect regularity to indefinitely large lengths (see Supplementary Movie 1). Although these fibres appear for of order unity, they form closer to than the expected , suggesting that fibre formation is not completely captured by the tentative equilibrium reasoning used to define . To confirm this, we extrapolate the specific energy of our periodic fibres to infinite lengths and compare them to that of the hexagon bulk shown in Figs 1c and 4a. As shown in Fig. 4b, the fibre energy exceeds that of the bulk, implying that fibres are indeed out of equilibrium.

We rationalize fibre formation by contrasting the marginal cost of adding a polygon to the side or to the tip of a pre-existing anisotropic aggregate (Fig. 2d). Upon a side addition, the new polygon is tucked into the existing structure, minimizing the surface energy cost associated with the addition. A tip addition, on the other hand, hardly deforms the existing aggregate and thus implies a lower deformation cost. This difference in deformation cost is more dramatic for thicker aggregates, where a side addition deforms a larger number of particles. As a result, for moderate surface tensions, side additions may be favourable for thinner aggregates but not for thicker ones, leading to the formation of finite-width fibres. As this argument specifically deals with marginal addition energies in sequential growth, it does not imply that fibres are global energy minima for the aggregate morphologies.

To confirm that our fibres are metastable aggregates, we next establish that they are unaffected by small perturbations in the growth pathway but change morphology if nucleated from a more stable phase. To test the first point, we modify our algorithm to successively add two polygons, then remove one. Similar to polygon addition, our polygon removal procedure minimizes the aggregate energy in a short-sighted fashion, allowing the relaxation of built-up stresses and thus lowering the aggregate energy. The whole procedure is then iterated until an aggregate of the desired size is obtained. As expected, fibres are essentially unaffected by this local change in protocol (Fig. 3b). We next grow an aggregate from a nucleus of the bulk, inducing significant morphological changes, as predicted (Fig. 3c). However, the one-dimensional, periodic growth is preserved, attesting to the robustness of the fibre-forming mechanism. Furthermore, seeding aggregates with fibre fragments results in morphologies identical to those of Fig. 3a (see Supplementary Information).

Moving beyond the *k* = 2 hexagons considered above, Fig. 3d, e demonstrates that our description is valid for a broad range of *k* corresponding to variations of the frustration energy *e*_{b} − *e*_{g} by several orders of magnitude, from ≃7 × 10^{−6} for *k* = 1.01 to ≃2 × 10^{−1} for *k* = 4. Despite these very substantial differences, the rescaled parameter remains an excellent predictor of fibre formation. Finally, we move away from hexagons altogether in Fig. 3f, g and demonstrate fibre formation in regular pentagons and octagons, two further shapes that do not tile the plane and thus generate intrinsically frustrated aggregates. Despite very diverse internal fibre structures, the onset of fibre formation is again very well predicted by the criterion .

Our results demonstrate that inherently frustrated aggregates of mismatched particles assume a richer range of morphologies than is found in well-matched objects. Moreover, they robustly form fibres when particle adhesion is commensurate with frustration, in strong contrast with the three-dimensional morphologies resulting from, for example, the flocculation of simple spherical colloids. Our analysis suggests that slender aggregates result from a compromise between, on the one hand, the elastic incentive to place all particles in the vicinity of the boundary of the aggregate to relax their frustrated shapes, and on the other hand, the tendency to form a compact aggregate that maximizes adhesion. This simple principle should also apply to three-dimensional objects, where the deformation cost illustrated in Fig. 2d is augmented by chirality effects, which favour one-dimensional twisted ribbons morphologies in colloidal assemblies^{10}. Moreover, chirality penalizes bulk aggregates in three dimensions^{11,12}, which can lead to the formation of either fibres or sheets.

The currently dominant paradigm for frustration in soft matter equates shape incompatibility with a mismatch between an intrinsically curved Riemannian metric favoured by the object and the flat metric of the embedding space^{13,14,15,16}. At equilibrium, this mismatch is accommodated by introducing defects in the system^{17} or by forming slender morphologies if defects are strongly penalized^{12,18,19,20,21}. Although slender morphologies and topological defects both arise in our aggregates (see Fig. 4c), our fibres are distinctively out-of-equilibrium structures. Moreover, they arise irrespective of whether the intrinsic Gaussian curvature of their constitutive polygons is positive (for pentagons), negative (octagons), or zero (irregular hexagons), in contrast to existing Riemannian metric models.

Turning to pathological fibre formation, our results suggest that the distinctive fibrous morphologies of protein aggregates need not be due to a mere coincidental convergence of molecular mechanisms, but could instead result from generic physical principles. Indeed, while the formation of cross-*β* spines is often discussed as the defining feature of one important class of such fibres, namely amyloids^{4}, deviations from this specific molecular organization have been observed^{22} and secondary interactions contribute significantly to their mechanics^{23} and morphologies^{24}. Although our simple model does not incorporate important effects such as the stochasticity due to thermal agitation or the entropic stabilization of fibres through their vibrational modes, these basic features are still consistent with the diverse morphologies we obtain upon small variations of our parameters, and could apply to protein fibres with radically different structures^{3}. Beyond biological materials, fibre formation upon aggregation could become a hallmark of self-assembled, frustrated matter, leading to new design principles taking advantage of increasingly sophisticated artificial asymmetrical building blocks at the nano- and microscale^{25,26}.

## Methods

### Expression of the aggregate energy.

The deformation energy for the *α*th polygon is a function of its area *A*^{(α)} and of the lengths {*ℓ*_{i}^{(α)}}_{i=1…n} of its sides through where *n* is the number of sides of the polygon. In this expression, the tendency to extend the area of the polygon due to the first term is counteracted by the harmonic restoring forces due to the second term (Fig. 2b). The elastic ground state of energy *e*_{g} discussed in the text is obtained by minimizing *e*^{(α)} with respect to the positions of the polygon’s vertices. Ground-state polygons are rigid, that is, devoid of internal soft modes due to the prestress inherent to equation (1) (ref. 27). The irregularity of this ground state can be continuously tuned through the choice of the spring constants *k*_{i}, and regular polygons are obtained when they are all identical. The alternating-side polygons presented in Figs 1b and 2a and used throughout have *k*_{1} = *k*_{3} = *k*_{5} = 1 (long sides, marked by pink tabs) and *k*_{2} = *k*_{4} = *k*_{6} = *k* > 1 (short sides, unmarked), which defines the asymmetry parameter *k*. Throughout this work we concentrate on the domain *k* ≥ 1 without loss of generality. Indeed our problem is invariant under the transformation *k* → 1/*k* by way of a proper rescaling of lengths and energies, and thus the aggregation process at any *k* ∈ (0,1) can be inferred from the appropriate *k* ∈ (1, *∞*). Although the specific form of the energy equation (1) is chosen for numerical convenience, its precise expression does not strongly influence our results.

Multiple polygons can be connected through the joining of one or several of their sides. Two joined sides are treated as a single object, implying that they share the same two end-vertices (Fig. 2a). We refer to the specification of all such junctions as the topology of the aggregate. The specification of a constrains the aggregate shape, and thus tends to increase the deformation energy *e*^{(α)} of each polygon above *e*_{g}. In this paper, we consider aggregates whose energies are minimal with respect to the position of their vertices for a given , and denote by the deformation energy of particle *α* in this state of mechanical force balance. We denote by the number of unjoined sides in topology ; for instance *N*_{u} = 10 in Fig. 2a, as indicated by the orange lines. Imposing the surface tension energy penalty *σ* > 0 to each unjoined side regardless of its actual length, the total energy of an aggregate comprising *N* polygons thus reads The first term of the right-hand side of equation (2) describes the total deformation energy in excess of the ground-state energy *Ne*_{g}, while the second term is the surface energy. Overall, *E* depends on the structure of the aggregate only through its topology . The average energy per particle discussed in the text is defined as *e* = *E*/*N*.

### Surface energy for trees and bulks.

We compute the surface energy of a tree comprising *N* polygons by noting that it has *N*_{u} = 2 + *N*(*n* − 2) unjoined sides. We demonstrate this by recursion over *N*, noting that *N*_{u} = *n* for *N* = 1. Each additional polygon adds *n* sides to the existing aggregate, *n* − 1 of which are unjoined. The existing aggregate also loses one unjoined side to the connection with the new polygon. Thus, *N*_{u} is incremented by *n* − 2 each time a new polygon is added to the tree, which proves our statement. The number of unjoined sides in a tree is thus proportional to its total number of polygons. As the number of unjoined sides in a two-dimensional bulk is proportional to , in the *N* → *∞* limit its surface energy is negligible compared to its nonzero elastic energy per particle.

### Deformation energy for trees and bulks.

The deformation energy of trees and bulks are computed by minimizing the energy equation (1) respectively with free boundary conditions or assuming the lattice structures illustrated in Fig. 4a for regular pentagons: regular octagons: and irregular hexagons: with and .

### Sequential aggregation algorithm.

We use a deterministic algorithm that considers all possible options for the addition of a polygon onto an existing aggregate, some of which are illustrated in Supplementary Fig. 4. After minimizing the total energy of the whole aggregate with respect to the coordinates of all its vertices for each option (which induces the polygon distortions seen in the figure), it selects the option associated with the lowest total energy *E* and uses the result as the basis of the next polygon addition. Similar to kinetic, irreversible protein aggregation *in vivo*, this procedure does not necessarily achieve the most energetically favourable aggregate topology globally. Instead, our algorithm locally guarantees the best energetic choice at each addition step, allowing the formation of metastable aggregates characteristic of our frustrated interactions.

### Data availability.

The data that support the plots within this paper and other findings of this study are available from the corresponding author upon request.

## Additional Information

Publisher’s note: Springer Nature remains neutral with regard to jurisdictional claims in published maps and institutional affiliations.

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## Acknowledgements

We thank R. Ball for a seminal conversation that inspired this work. We are also grateful to E. Efrati for his insights on the connection between frustration and intrinsic curvature, and for suggesting our initial fibre-forming realization using pentagons. We thank him and P. Ronceray for comments on the manuscript. This work was supported by grants from Université Paris-Sud’s Attractivité and CNRS’ PEPS-PTI programmes, Marie Curie Integration Grant PCIG12-GA-2012-334053, ‘Investissements d’Avenir’ LabEx PALM (ANR-10-LABX-0039-PALM), ANR grant ANR-15-CE13-0004-03 and ERC Starting Grant 677532. This work was also supported in part by the National Science Foundation’s MRSEC Program under Award Number DMR-1420709. ML’s group belongs to the CNRS consortium CellTiss.

## Author information

## Affiliations

### LPTMS, CNRS, Univ. Paris-Sud, Université Paris-Saclay, 91405 Orsay, France

- Martin Lenz

### Department of Physics and James Franck Institute, University of Chicago, Chicago, Illinois 60637, USA

- Thomas A. Witten

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### Contributions

M.L. and T.A.W. designed the research and wrote the manuscript. M.L. performed the research.

### Competing interests

The authors declare no competing financial interests.

## Corresponding author

Correspondence to Martin Lenz.

## Supplementary information

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### Supplementary information

Supplementary information

## Videos

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### Supplementary movie

Supplementary movie 1