Modulated nematic structures induced by chirality and steric polarization

Modulated nematic structures induced by chirality and steric polarization

Lech Longa Marian Smoluchowski Institute of Physics, Department of Statistical Physics, Jagiellonian University, Łojasiewicza 11, Kraków, Poland    Grzegorz Paja̧k Marian Smoluchowski Institute of Physics, Department of Statistical Physics, Jagiellonian University, Łojasiewicza 11, Kraków, Poland
July 5, 2019

What kind of one-dimensional modulated nematic structures (ODMNS) can form nonchiral and chiral bent-core and dimeric materials? Here, using Landau-deGennes theory of nematics, extended to account for molecular steric polarization, we study a possibility of formation of ODMNS, both in nonchiral and intrinsically chiral liquid crystalline materials. Besides nematic and cholesteric phases, we find four bulk ODMNS for nonchiral materials, two of which have not been reported so far. These new structures are longitudinal () and transverse () periodic waves where the polarization field being periodic in one dimension stays parallel and perpendicular, respectively, to the wave vector. The other two phases have all characteristic features of the twist-bend nematic phase () and the splay-bend nematic phase (), but their fine structure appears more complex than that considered so far. The presence of molecular chirality converts nonchiral and into new phases. Interestingly, the nonchiral phase can stay stable even in the presence of intrinsic molecular chirality. Exemplary phase diagrams provide further insights into the relative stability of these new modulated nematic structures.

Until very recently only four classes of nematics were recognized: (i) uniaxial and (ii) biaxial nematics for nonchiral liquid crystalline materials and (iii) cholesteric and (iv) blue phases for chiral liquid crystals deGennesBook (). The most surprising recent discovery is the identification of the fifth. In this new phase, found in liquid crystalline systems of chemically achiral dimers PanovNTB (); CestariNTB (); BorshchNTB (); ChenBananyPNAS (), bent-core mesogens GleesonGoodby (); ChenBananyPRE2014 () and their hybrids hybridbentcores (), the molecules are arranged to form a helical superstructure with nanoscale periodicity. This periodicity is about two orders of magnitude shorter than typically found in cholesteric and blue phases of ordinary chiral materials. As the molecular centers of mass are distributed randomly in space the structure belongs to the nematic class. It coined the name twist-bend nematic phase (). Contrary to cholesterics, the director in is not perpendicular to the helix axis, but precesses on a cone, with the helical axis parallel to the cone’s axis. As formation of does not require any presence of molecular chirality experimentally coexisting domains of opposite chirality are observed. So far the phase is stabilized below uniaxial nematic phase () as a result of first order phase transition on the temperature scale. Hence, we observe a fundamentally new phenomenon namely the spontaneous chiral symmetry breaking within the nematic class of materials.

Very recently, chiral asymmetric dimers were also studied ZepGoreckaChiralSB (); Gorecka2015 (). Here the intrinsic molecular chirality is an extra factor giving rise to overall a sequence of up to seven distinct nematic phases. As the constituent molecules are intrinsically chiral the highest-temperature phase is the cholesteric phase () or a blue phase. Stable phases observed at lower temperatures are variants of with pitch which is larger than one in achiral Gorecka2015 ().

The issue of stable and structures has been addressed at theoretical level in two important papers MeyerFlexopolarization (); DozovNTB (). With the aid of symmetry arguments, supplemented by second-order elasticity theory of the director field, Meyer MeyerFlexopolarization () and later on Dozov DozovNTB (), have analyzed some consequences of spontaneous local bend or splay deformations of the nematic director on the polar organization of the molecules - the so called flexoelectric effect. While the cholesterics can fill the space with homogeneous twist it appears that the corresponding bend state should always be associated either with some twist or splay. According to this picture the uniform nematic phase would then become unstable to the formation of a modulated phase, which could be either or DozovNTB (). A prerequisite to such behaviour would be the sign change of the (effective) bend Frank elastic constant, . Indeed, determined experimentally in BorshchNTB (); AdlemLuckhurstNTB () is anomalously small as the transition to is approached.

Recently, Shamid et al. SelingerNTB2013 () have developed Landau theory and lattice simulations of polar order and director bend deformations, correlating flexoelectricity, negative and stability of and phases. They predicted a second-order phase transition from high-temperature N phase to low-temperature or . At the transition, the effective changes sign and the corresponding structure develops modulated polar order, averaging to zero globally. All phases are assumed uniaxial and described entirely using director and polarization fields.

The purpose of this Letter is to investigate how nematics can self-organize into ODMNS for nonchiral and intrinsically chiral V-shaped molecules, using first-principles, symmetry-based generalization of Landau-deGennes theory of nematics. We assume that the second-rank traceless and symmetric alignment tensor field, , is the primary order parameter accounting for nematic order deGennesBook (). It permits that locally a system is described by a tripod of orthonormal directors and corresponding eigenvectors . Identifying the full biaxial field with primary order parameter of nematics, rather than its -part only DozovNTB (), should also clarify whether biaxiality () is relevant for , for we know that chiral nematic phases of at least intrinsically chiral mesogens are all biaxial lechChiralIcosa (). Important theoretical questions are thus about structure characterization of ODMNS, both for non-chiral and intrinsically chiral materials ZepGoreckaChiralSB (); Gorecka2015 ().

For the modeling of spontaneous chiral symmetry breaking as observed in the -tensor alone is not sufficient. In the lowest order scenario we need, in addition to , at least one secondary order parameter, which can be either a first-rank (polar) field, lechChiralFlexo (), or a third-rank tensor field , invariant with respect to tetrahedral point group symmetry FelTetrahedratic (); multitensor (); BrandTetrahedratic (); longaTetra2009 (); tetraDuality (); longaTetra2012 (); longaTetra2013APP (). The difference between these scenarios would be the polar order for and couplings lechChiralFlexo () and lack of polarity but the presence of nonlinear dielectric tensor for and . Here we focus on one-dimensional modulated structures as induced by and . We look systematically into extended Landau-deGennes-Ginzburg (LdeG) free energy expansion and discuss the role played by various symmetry-allowed, lowest-order couplings. The essential ordering mechanism towards one-dimensional modulated structures will then be identified with the help of bifurcation and numerical analyses.

Before we proceed further it is important to realize that the polar field, , does not need to be of electrostatic origin. Bend-core molecules are primarily polar due to their ”V” shape while bimesogens acquire steric polarization in their conformational states. Such steric dipoles are present even in the absence of electrostatic dipoles. In a densely packed environment, we expect that these entropic, excluded volume interactions, rather than charge moments, define the local order, such as . Recently, Greco and Ferrarini have studied systems composed of crescent-shaped molecules interacting through a purely repulsive potential providing strong support for entropy-driven transition 2015prlGreco ().

We start by introducing the minimal coupling, LdeG free energy per volume, constructed as a power-series expansion in and , and their derivatives. It can be decomposed as


where are the free energy densities constructed out of the order parameters and contributing to in th order. By taking suitable units of energy, length, and and disregarding electric field, magnetic field and surface terms the general form of up to fourth-order in can be written as


where, as usual, is the reduced temperature associated with ; is the reduced chirality, proportional to the wave vector of the cholesteric phase and is the relative elastic constant. Likewise, the polar parts are


Clearly, for electric dipoles would vanishes in (4,5) while the -term should be replaced by direct interactions between charge distributions. However, for purely steric dipoles, associated with excluded volume interactions 2015prlGreco () these terms are all present. In particular, for intrinsically chiral materials that develop steric polar order the chiral parameters , and are all nonzero.

General, orientational properties of polar biaxial liquid crystals, characterized by and , were analyzed in lechElastic1 (); lechChiralFlexo (). In particular the flexopolarization couplings were identified and classified. Assuming deformations to appear only in a quadratic part of the free energy and neglecting surface terms the lowest-order cross-coupling terms are


The LdeG expansion (2-7) is the minimal coupling theory for systems described in terms of and , where is of steric origin. Our objective is to identify possible ODMNS that minimize for arbitrary and , and for fixed values of the material parameters. By taking we assume from the start that is secondary order parameter. A brief account of what to expect from such theory has already been presented long ago in lechChiralFlexo (), where we indicated on a possibility of flexopolarization-induced periodic, one-dimensional structures. A more quantitative analysis of modulated nematic structures that can be driven by (flexo-)polarization is found in AlexanderFlexoBP (); SelingerPolarBluePhases2014 (); MishaNTB&NSB (). In their theory Alexander and Yeomans AlexanderFlexoBP () showed that applying an electric field to a sample with a large flexoelectric response can stabilize and a flexoelectric blue phase. Shamid, Allender and Selinger SelingerPolarBluePhases2014 (), on the other hand, have taken a simpler version of the expansion lechChiralFlexo () and showed that the system can stabilize a polar analogue of chiral blue phases if polar order is allowed to be induced spontaneously.

In this letter we study inhomogeneous nematics with inhomogeneity propagating in one spatial direction, both for nonchiral and intrinsically chiral materials. We show that modulated phases, identified so far as a result of polar coupling, do not exhaust all possibilities that the theory (1-7) allows for. Our ultimate goal will be to look into fine structure of these phases and clarify the role played by biaxiality. In order to address these issues we explore the bifurcation theory supplemented by numerical minimization and identify global minima of , Eq. (1), within the ODMNS family, leaving a more complex issue of stable blue phases to our future studies.

The above programme is realized in practice by expanding and into plane waves of definite helicity: , Here are wave-vectors, and are the variational parameters in the free energy expansion, and , , , , and finally are the spin spherical tensors represented in an orthonormal, right handed local coordinate system with as quantization axis. Two amplitudes of opposite helicity out of , can be taken real due to invariance of and with respect to uniform translations in 3D and global rotations about . We choose . The reality condition: additionally implies that and . The selection of and relevant amplitudes , is fixed by the bifurcation analysis longajcp (); longaBif () while their numerical values are found by the subsequent minimization of .

In the vicinity of the isotropic phase the dominant contributions to , Eq. (1), comes from which, for the ODMNS structures, is




Here is replaced by , by and by ; is the Kronecker delta. Setting determines the equilibrium value of the amplitudes and -vector for given material parameters. Since explicit dependence on appears only in second-order contributions, we have . Note that the -terms linear in promote modulated structures, among which are ODMNS. As it turns out an interesting class of ODMNS can already be identified by studying a simpler model where . In what follows we shall consider this simpler case leaving analysis of the full model, along with the issue of stable blue phases, to our forthcoming publications. In addition we take and . For thermodynamic stability it is also necessary that and . Additionally, must be positive if .

We shall now proceed by analyzing the case of and later discuss the effect of . For the first-mentioned case the polarization field appears only in and, hence, the condition can be solved for given fixed . It yields


Substituting (10) back to we obtain the effective free energy that still has to be minimized with respect to . Only is modified by this substitution. It reads


Note that the leading elastic part of can again be cast in form (2), but with being replaced by . Since vanishes for twist deformations lechElastic1 () the flexopolarization must induce splay-bend instability for . However, the term alone cannot bring about spontaneous chiral symmetry breaking. For that we need sufficiently large .

We shall now seek for ODMNS that can be stabilized as result of a phase transition from the isotropic phase. The general method is to analyse the nonlinear equations for the amplitudes and using the bifurcation analysis (BA) longajcp (); longaBif (). We apply this method to identify the leading amplitudes in the expansion of and close to a phase transition from the isotropic phase (), where , to an ordered ODMNS. The procedure is straightforward for . In the zeroth-order of BA the amplitudes are close to their isotropic values and, hence, governed by the part of . Since is in its diagonal form we can identify five different ODMNS, each characterized by the single mode of helicity , that bifurcate from at temperatures , where equals to at which the coefficient in front of in Eq. (11) vanishes. The corresponding wavectors, , are determined from with given by Eq. (10). The maximal of the temperatures represents a potential transition temperature from to ODMNS for a continuous phase transition and spinodal for a first order phase transition. Explicitly, the modes bifurcate from when and . The condensation of modes occurs when and satisfy the implicit relations and They can be resolved for non-chiral materials () giving and , which are satisfied for . Finally, and , for . We should mention that the bifurcation from to takes place at . First-order BA, consistent with modelling of the phase lechChiralIcosa (), allows to identify the next to leading amplitudes of ODMNS that couple to those given above through and . A subsequent minimization of either with respect to so identified trial states or with respect to all amplitudes of gives (consistently) six different ODMNS, shown in Fig. 1.

Our numerical minimization is carried out for the exemplary sets of material parameters. The corresponding phase diagrams are shown in Figs (2-5). The bifurcation temperatures from the isotropic phase are also plotted as dashed lines. All phase transitions involved are at least weakly first order although with increasing and decreasing the difference between the bifurcation- and transition temperatures becomes numerically negligible.

Figs (2,3) show new ODMNS structures predicted by the model for . These flexopolarization-induced nonchiral structures are referred to as and . In the polarization vector, Fig. (1), is always perpendicular to and , and . The homogeneous nematic background (, ) makes locally biaxial with biaxiality modulated along . The phase is constructed out of modes. Here and are always parallel to . The phase is uniaxial and periodically changes between prolate and oblate. In order to obtain the transition from to the term, (Eq.8), should be small positive or negative. In the phase an inhomogeneous biaxial modulation is also generated. Here is periodically modulated in the ,-plane of splay-bend deformations.

Figure 1: (Color online) ODMNS predicted by the theory (leading nonzero amplitudes are given in braces): , , , , , , , as in , as in , , , as in and , . Lengths of cuboid edges are proportional to the moduli of eigenvalues of . Red arrows represent and black arrow is the direction of .
Figure 2: (Color online) Phase diagram for , , , and . Solid lines are obtained from numerical minimization while dashed curves are bifurcation temperatures from the isotropic phase.
Figure 3: (Color online) Phase diagram for , , , and . For further details see caption to Fig. 2.

The phase diagrams presented in Figs (4-5) show changes induced by intrinsic molecular chirality for . Clearly, results in replacing by , where and rotates about and remains everywhere perpendicular to . Changes also concern and . transforms into , Fig. 1, which is biaxial with precessing on the cone about and parallel to and perpendicular to . The phase is also biaxial, where two out of the three directors posses twist deformations similar to the ones modelled in MishaNTB&NSB (). in this phase is a linear combination of all three directors. Interestingly, the nonchiral phase can become stable even in intrinsically chiral materials, Fig. (5).

Figure 4: (Color online) Phase diagram for , , , and . Here all modulated phases are chiral. For further details see caption to Fig. 2.
Figure 5: (Color online) Phase diagram for , , , and . Despite nonzero intrinsic chirality there is a stable region of achiral modulated structure. For further details see caption to Fig. 2.

The phase can be stabilized not only for , but primarily when . In order to obtain the phase for nonchiral materials the sign of must be consistent with the sign of and should exceed a threshold value. For example, if we take parameters of Fig. 2 and , the phase becomes stable for . Calculations carried out for show rich sequence of phase transitions: , where phases in parentheses are optional. Although the phases obtained for (a) and (b) have the same symmetry, in the first case the structure of helicity minimizes , while for the case (b) structures of opposite helicities are of the same free energy, which is know as ambidextrous chirality. The cases (a) and (b) differ quantitatively, i.e. in periodicities and biaxiality parameter lechChiralIcosa ().

In conclusion, LdeG phenomenological theory of nematics extended to account for molecular steric polarization, stabilizes four bulk ODMNS for nonchiral materials, two of which: and have not been reported so far. The presence of molecular chirality converts into and into new chiral , but the nonchiral phase can stay stable even in the presence of intrinsic molecular chirality.

The authors thank Misha Osipov for stimulating discussions. This work was supported by the Grant No. DEC-2013/11/B/ST3/04247 of the National Science Centre in Poland.


  • (1) P. G. de Gennes and J. Prost, ”The Physics of Liquid Crystals” (2nd edition, Clarendon Press, 1993).
  • (2) V. P. Panov et al., Phys. Rev. Lett. 105, 167801 (2010).
  • (3) M. Cestari et al., Phys. Rev. E 84, 031704 (2011).
  • (4) V. Borshch et al., Nat. Commun. 4, 2635 (2013).
  • (5) D. Chen et al., PNAS 110, 15931 (2013).
  • (6) V. Görtz et al., Soft Matter 5, 463 (2009).
  • (7) D. Chen et al., Phys. Rev. E 89, 022506 (2014).
  • (8) Y. Wang et al., CrystEngComm 17, 2778 (2015).
  • (9) A. Zep et al., J. Mater. Chem. C 1, 46 (2013).
  • (10) E. Gorecka, et al., Angew. Chem. Int. Ed. 54, 10155 (2015).
  • (11) R. B. Meyer, pages in ”Proceedings of the Les Houches Summer School on Theoretical Physics, 1973, session No. XXV” edited by R. Balian and G.Weill (Gordon and Breach, 1976).
  • (12) I. Dozov, Europhys. Lett. 56, 247 (2001).
  • (13) K. Adlem et al., Phys. Rev. E 88, 022503 (2013).
  • (14) S. M. Shamid et al., Phys. Rev. E 87, 052503 (2013).
  • (15) L. Longa et al., Phys. Rev. E 50, 3841 (1994).
  • (16) L. Longa and H.-R. Trebin, Phys. Rev. A 42, 3453 (1990).
  • (17) T. C. Lubensky and L. Radzihovsky, Phys. Rev. E 66, 031704 (2002).
  • (18) L. G. Fel, Phys. Rev. E 52, 702 (1995).
  • (19) H. R. Brand et al., Physica A 351, 189 (2005).
  • (20) L. Longa, G. Paja̧k and T. Wydro, Phys. Rev. E 79, 040701(R) (2009).
  • (21) L. Longa and G. Paja̧k, Mol. Cryst. and Liq. Cryst. 541, 152 (2011).
  • (22) K. Trojanowski et al., Phys. Rev. E 86, 011704 (2012).
  • (23) L. Longa and K. Trojanowski, Acta Phys. Pol. B 44, 1201 (2013).
  • (24) C. Greco and A. Ferrarini, Phys. Rev. Lett. 115, 147801 (2015).
  • (25) L. Longa, D. Monselesan and H.-R. Trebin, Liq. Cryst. 6, 769 (1987).
  • (26) G. P. Alexander and J. M. Yeomans, Phys. Rev. Lett. 99, 067801 (2007).
  • (27) S. M. Shamid et al., Phys. Rev. Lett. 113, 237801 (2014).
  • (28) N. Vaupotič et al.,Phys. Rev. E 89, 030501(R) (2014).
  • (29) L. Longa, J. Chem. Phys. 85, 2974 (1986).
  • (30) L. Longa et al., Phys. Rev. E, 71, 051714 (2005).
Comments 0
Request Comment
You are adding the first comment!
How to quickly get a good reply:
  • Give credit where it’s due by listing out the positive aspects of a paper before getting into which changes should be made.
  • Be specific in your critique, and provide supporting evidence with appropriate references to substantiate general statements.
  • Your comment should inspire ideas to flow and help the author improves the paper.

The better we are at sharing our knowledge with each other, the faster we move forward.
The feedback must be of minimum 40 characters and the title a minimum of 5 characters
Add comment
Loading ...
This is a comment super asjknd jkasnjk adsnkj
The feedback must be of minumum 40 characters
The feedback must be of minumum 40 characters

You are asking your first question!
How to quickly get a good answer:
  • Keep your question short and to the point
  • Check for grammar or spelling errors.
  • Phrase it like a question
Test description