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The electroclinic effect and modulated phases in smectic liquid crystals


The electroclinic e?ect and modulated phases in smectic liquid crystals
Robert B. Meyer
The Martin Fisher School of Physics, Brandeis University, Waltham, Massachusetts 02254-9110

Robert A. Pelcovits

arXiv:cond-mat/0202184v2 [cond-mat.soft] 25 Feb 2002

Department of Physics, Brown University, Providence, RI 02912 (Dated: February 1, 2008) We explore the possibility that the unusually large electroclinic e?ect observed in the smectic–A phase of a ferroelectric liquid crystal arises from the presence of an ordered array of disclination lines and walls in a smectic–C ? phase. If the spacing of these defects is in the subvisible range, this modulated smectic–C ? phase would be similar macroscopically to a smectic–A phase. The application of an electric ?eld distorts the array, producing a large polarization, and hence a large electroclinic e?ect. We show that with suitable elastic parameters and su?ciently large chirality, the modulated phase is favored over the smectic–A and helically twisted smectic–C ? phases. We propose various experimental tests of this scenario.
PACS numbers: 61.30.Cz, 61.30Gd, 61.30Mp

I.

INTRODUCTION

Chiral liquid crystals exhibit a variety of interesting phenomena [1]. Chiral molecules tend to pack at a slight angle with respect to their neighbors. This preferred packing leads to spontaneous twist in the molecular orientation, producing phases such as the cholesteric and helically twisted smectic–C ? (Sm–C ? ). In the case of two–dimensional Sm–C ? ?lms, the chiral modulation of the molecular orientation cannot occur in a defect–free fashion. Instead, for large chirality, the system will form a modulated phase consisting of a regular network of defect walls and possibly points. One possible modulated phase is a “striped” phase consisting of a regular array of parallel domain walls (Fig. 1). In between these walls the c director rotates in the sense preferred by the chirality. Another possible modulated phase consists of a hexagonal array of domain walls, with point defects located at the centers and corners of the hexagonal cells (Fig. 2). Chirality also leads to unusual e?ects in orientationally disordered phases. As shown by Garo? and Meyer [2] using symmetry arguments, if an electric ?eld is applied to a system of chiral molecules in the Sm–A phase, an average molecular tilt will be produced, a response termed the electroclinic e?ect. These symmetry arguments do not, however, indicate the microscopic basis of the electroclinic e?ect. To date, two microscopic models have been proposed. In the ?rst, the long axes of the molecules are assumed to be perpendicular to the smectic layers in the Sm–A phase. The electric ?eld causes the molecules to tilt, with an accompanying signi?cant change in the smectic layer spacing. In the second scenario suggested by de Vries [3], the molecules in the Sm–A phase are assumed to be tilted even in the absence of the electric ?eld, but azimuthally disordered. The electric ?eld then induces azimuthal order, with no signi?cant change in the smectic layer spacing. Experimental studies have shown evidence for both models, at least

FIG. 1: Striped modulated phase in a thin Sm–C ? ?lm. The circular heads of the objects shown denote the heads of the local c director; the vertical lines are domain walls where the c director rotates by an angle of order π.

2

FIG. 2: Hexagonal modulated phase in a thin Sm–C ? ?lm. There is a +1 disclination at the center of each unit cell, and ?1/2 disclinations at each corner. Domain walls where the c director rotates by an angle of order π bound the cell.

in terms of the ?eld–induced layer contraction. Recently Selinger et al. [4] noted that the optical birefringence of the liquid crystal will also distinguish between the two microscopic pictures. Because the ?eld induces orientational order in the second model while simply tilting the already aligned molecules in the ?rst, the birefringence should change dramatically in the former model, but not the latter. It appears that each of these models has experimental validity, namely there are materials with substantial layer contraction and weak ?eld dependence in the birefringence, and other materials with the opposite properties. However, even a detailed theory based on the second model [4] is unable to fully describe the experimental data. Furthermore, many materials show an unusually large electroclinic e?ect, well into the Sm–A phase. While it is tempting to associate this large e?ect with strong critical ?uctuations [4], a completely di?erent molecular mechanism may be relevant. In this paper we propose a new model for the microscopic origin of the electroclinic e?ect, one that shares some of the macroscopic characteristics of the de Vries scenario, speci?cally, no layer contraction and ?eld dependent birefringence. We postulate that what is assumed to be a Sm–A phase in some materials close to the Sm–C ? ? A transition, could in fact be a modulated version of the smectic–C ? phase, a network of defects, walls and lines, but one where the spacing between the defects is in the subvisible range. This modulated phase would have no long–range azimuthal order or net polarization in the absence of an electric ?eld. Thus, “to the eye”, this phase would appear to be a Sm–A phase. However, the application of an electric ?eld distorts the structure of the defect array and leads to a large electroclinic e?ect. We now describe our proposed modulated phase and its response to an electric ?eld in detail. A bulk chiral Sm–C ? can be described by the following elastic free energy [5]: F = + d3 x 1 1 1 K1 (? · c)2 + K2 (c · ? × c + q)2 + K13 (? · ? × c)(c · ? × c) z 2 2 2 (1)

1 K3 (? · ? × c)2 ? w z · ? × c z ? 2

where c is the projection of the nematic director on the plane of the layers. We assume that the molecular tilt is uniform and thus c is assumed to be of ?xed length. Chirality appears in two terms in this free energy. First, chirality induces a spontaneous twist of the c director as indicated in the second term on the right hand side of Eq. (1), which is minimized in a helical state with pitch 2π/q. Second, chirality induces spontaneous bend within each smectic layer as indicated by the last term in the free energy, where we assume w > 0. The free energy as written is zero

3 for the perfect helical state with pitch 2π/q. Because the smectic–C ? phase is ferroelectric, with the spontaneous polarization perpendicular to c, we must add to this free energy an electrostatic term arising from space charge density proportional to z · ? × c. We ignore this term for now, since we will ?nd that in our proposed modulated phase, it ? adds only a constant to the free energy density, independent of the detailed structure of our model. Considerable work has been done on analyzing Eq. (1) in t wo–dimensional chiral smectic liquid crystals, where the terms proportional to K2 and K13 in the free energy above are absent, and thus, there will be no competition between the two chiral terms. While only one chiral term is present, it is impossible to impose a spontaneous bend throughout the system. Defects must be introduced which separate domains of spontaneous bend, thus leading to a modulated phase. Two types of modulated phases have been proposed, a “striped” phase (Fig. 1) with a one–dimensional modulation [6, 7, 8], and a hexagonal phase (Fig. 2) with a two–dimensional modulation. In the former case, parallel domain walls separate regions of spontaneous bend, while the latter consists of a two–dimensional array of domain walls and point disclinations. A +1 point disclination lies at the center of each hexagonal cell, while the boundaries of the cell are domain walls where the c director rotates by π (a description of internal structures of these walls in terms 1 of a non?xed length c director ?eld is given in [7, 8]). A ? 2 point disclination is located at each corner of the cell. The hexagonal phase which involves nearly pure bend is favored over the striped phase when K1 ? K3 . The size of the unit cell is inversely proportional to the strength of the chirality parameter w. The free energy of the hexagonal lattice includes (see Eq. (5) below) an attractive logarithmic interaction between the +1 disclination at the center of the cell and the ? 1 disclinations at the corners. Thus, strongly chiral materials, where the unit cell is small, will 2 favor this interaction, and hence the hexagonal phase [1]. Returning to the full three–dimensional free energy, Eq. (1), we consider the possibility of a modulated phase. A bulk modulated phase must somehow compromise between the two competing chirality–induced tendencies: spontaneous in–layer bend and spontaneous twist about the layer normal. To describe the electroclinic e?ect in our proposed scenario the bulk modulated phase must have zero net polarization. Thus, a bulk modulated phase produced by simply extending the two–dimensional striped phase in the third direction is not acceptable, even if the pitch of the spontaneous twist were assumed to be in?nitely large. A three–dimensional model for a thick chiral smectic ?lm was proposed in Ref. [9], where the in–plane modulation and domain walls are con?ned to surface regions, and the director twists in the interior of the ?lm. Here we consider a space–?lling modulated structure, with no need for surface structures. Our starting point in constructing a suitable bulk modulated phase is the director con?guration of the +1 point disclination at the center of the two–dimensional hexagonal cell (Fig. 2). Expressing the c director as c = (cos θ(x, y), sin θ(x, y)), the angle θ is given by: θ(x, y) = φ(x, y) + φ0 , (2)

where the polar angle φ(x, y) is given by φ(x, y) = arctan (y/x), and φ0 = π/2 (for the sign of the chirality appropriate to the structure shown in Fig. 2; for the opposite sign of chirality, φ0 = ?π/2, and the director circulation will be clockwise). This con?guration represents pure bend and describes the director con?guration away from the domain walls which bound the unit hexagonal cell. We now form a three–dimensional simple hexagonal lattice, with a unit cell of height h, and cross–sectional area as in the two–dimensional case. We specify the director con?guration as follows. In the midplane of the unit cell (taken to be the z = 0 plane) we assume the perfect bend director con?guration of Eq. (2). We then introduce twist in the z direction, by writing the angle θ(x, y, z) of the c director as follows: θ(x, y, z) = φ(x, y) + φ0 (z), with φ0 (z) = π/2 + πz/?, ?h/2 < z < h/2. (4) (3)

The pitch ? of this helical structure will be determined by minimizing the free energy density of the unit cell. With this model for the modulated phase, the K13 and w terms in the free energy, Eq. (1), can be combined into a term like the w term with wef f = w + π/?. We ?nd that ? is so large that for simplicity we set wef f = w. Thus the unit cell has a +1 disclination line running along the central z axis of the cell and parallel ?1/2 disclination lines along the edges of the cell. Within the cell the director twists along the z axis, in the sense preferred by the chirality (see Fig. 3). The top and bottom faces of the cell (perpendicular to the z axis) are domain walls where the director undergoes a rotation by 2πh/?. The six other faces of the cell are walls where the c director rotates by π. The free energy density of the hexagonal unit cell (of side R) relative to the helical state is given by:

4

FIG. 3: A slice through the bulk hexagonal lattice at z = ?/6, showing how the director has twisted by an angle of π/6 relative to the z = 0 slice shown in Fig. 2.

f=

2π 2πK ln(R/Ro ) + K ′ √ + K2 q ? 2 /2 ? 3 3R

2

?

2 ln 3w? 2AT 2AS , sin(πh/2?) + +√ πhR h 3R

(5)

where we have assumed that K1 = K3 = K to simplify the elastic energy expression associated with the disclination lines. The core size of the disclination lines is denoted by Ro , and we represent the domain wall energy per unit area of the top and bottom faces of the cell by AT , and the wall energy per unit area of each side face by AS . The term proportional to ln(R/a) includes the elastic energy per unit cell associated with the +1 disclination line at the center of the cell and the surrounding ?1/2 disclination [8]. The term K ′ represents the remainder of the splay–bend elastic energy per unit cell. The term proportional to w is obtained by integrating the corresponding term in Eq. (1) over the hexagonal unit cell using the director pro?le Eq. (3), thus ignoring the distortion of this pro?le near the edges of the cell. Before minimizing this free energy density we consider the response of the modulated state to an electric ?eld, i.e., the electroclinic e?ect. We assume that the direction of the molecular dipole moment p is given by c × z . In the ? two–dimensional hexagonal modulated phase (see Fig. 2), the molecular dipole moments near the center of the cell will point radially outward, given the bend con?guration of the c director. Thus, an electric ?eld applied in the +x direction will shift each +1 disclination in the opposite direction, inducing a net polarization in the +x direction, as shown in Fig. 4. For the three–dimensional cell we assume that the +1 disclination lines at the cell centers also shift rigidly in the opposite direction to the ?eld, ignoring any possible bending of the line due to the twist of the director in each cell (this should be a higher–order e?ect in the electric susceptibility). Assuming that the disclination lines shift by a distance d in the ?x direction, we ?nd that the polarization (the net dipole moment of a cell divided by its volume V ) is given to leading order in d by: 2dp?R sin(πh/2?), V a3

P =

(6)

where p is the molecular dipole moment and a is the average intermolecular spacing. In deriving P we have assumed that the unit cell is a cylinder of radius R centered on the original position of the line; ignoring the hexagonal shape of the cell merely changes the numerical prefactor appearing in the above expression.

5

FIG. 4: The z = 0 slice through the bulk hexagonal lattice in the presence of an electric ?eld in the +x direction. The arrows here represent the molecular dipole moments which are locally perpendicular to the c director and lie in the x ? y plane. The electric ?eld shifts the disclination line at the center of each cell to induce a net polarization in the direction of the ?eld.

The distance d is determined by minimizing the change in the free energy density due to the presence of the ?eld. Displacing the disclination line by a distance d costs elastic energy proportional to Kh(d/R)2 . Thus, d is given by: d= the polarization by: P ≈ and the susceptibility by: χP ≡ dP p2 ? 2 R 2 sin2 (πh/2?). = dE Ka6 h2 (9) p2 ? 2 R 2 E sin2 (πh/2?), Ka6 h2 (8) p?ER3 sin(πh/2?), Kha3 (7)

We now consider the minimization of f , which is a function of R, ?, and h. Minimizing ?rst with respect to R, we ?nd the following condition: R= where fW and
′ Ro = Ro exp

4πK ′ ln(R/Ro ), 3fW

(10)

√ w? 3 ln 3 = sin(πh/2?) ? AS , πh K′ 1 . ? 2 2πK

(11)

(12)

6
′ Eq.(10) has a solution for R > Ro providing fW > 0. This condition is physically equivalent [7] to requiring that the domain wall energy of the side walls of the cell be negative in a non–?xed length director model, where the wall energy includes surface contributions, i.e., contributions from the total gradient term ? × c. Numerical minimization of the free energy density, Eq. (5), with respect to R, ?, and h, (choosing K = K2 = 1, K ′ = AT = AS = 0.1) indicates that for values of w that yield f < 0, (i.e., when the modulated state is favored over the helical state), h ≈ 105 , ?/h ≈ 100, and:

2? sin(πh/2?) ≈ 1. πh

(13)

The condition ? ? h is sensible, because in that case the director pattern in each cell will be nearly pure bend. In √ this limit the condition fW > 0 implies that AS < w 3 ln 3/2 ≈ w. With ? very large, the polarization space charge density, proportional to z · ? × c varies in each cell as 1/r, with ? r the distance from the central disclination, and is almost independent of z. This produces an electric ?eld E which is almost purely radial, and constant in magnitude, considering the cell to be approximated by a cylinder. At the outer boundary of the cell there is a surface charge which precisely cancels the charge in the interior of the cell, so that there is no electric ?eld outside each cell due to the charge distribution within the cell and on its boundaries. Thus the electrostatic energy density can be evaluated in a single cell, and is proportional to E 2 , independent of the radius or height of the cell. Although there are also ionic charges present in liquid crystals, typical estimates of their screening length indicate that they would not alter the electric ?elds at the length scales we are considering. Assuming that ? is large, as indicated by the numerical minimization of Eq. (5), (speci?cally, ? ? q ?1 ), and using Eq. (13), the free energy density Eq. (5) can be approximated as: √ 2 ′ 3fW (2 ln(R/Ro ) ? 1) P2 . (14) f ≈ K2 q 2 + 0 ? 2 ′ 8π? 8πK ln (R/Ro ) in which the electrostatic term, with spontaneous polarization density P0 and dielectric constant ?, has been included. We determine R by numerically solving Eq. (10), using Eq. (13), and choosing K = 1, K ′ = AS = 0.1 and 2 K2 q 2 + P0 /(8π?) = 0.0025 ; the results are shown in Fig. 5. Using these results for R we obtain the approximate free energy density, Eq. (14), as a function of w (as shown in Fig. 6, choosing K2 = 1, AT = 0.1). We see that if w > 0.39, the hexagonal phase is favored over the helical state. The numerical minimization of the full expression ? for the free energy, Eq. (5), indicates that in this phase h ≈ 105 , in units of an intermolecular spacing. Thus, the hexagonal phase in a real system would likely consist of a single lattice plane of hexagonal cells, i.e., the system is e?ectively two–dimensional. From Eqs. (9) and (13) we see that: χP ? R 2 . We plot χP as a function of w in Fig. 7.
II. CONCLUSIONS

(15)

Returning now to the observations that motivated this work, we can see that if R is a sub-visible length, then the modulated phase would resemble a Sm–A phase, optically. In our model, the apparent Sm–A to Sm–C ? transition, as temperature is lowered, would actually be mimicked by the gradual change of physical parameters, so that below the transition temperature, the helical Sm–C ? phase would have lower free energy than the modulated phase. In our model, this would be a ?rst order transition. Since the driving term in the free energy density, Eq. (5), favoring the modulated phase is the term proportional to w, one could say that if w decreases as temperature is lowered while all other parameters remain constant, then when w passes through a particular value (about 0.39 in our calculated example) a ?rst order transition to the helical Sm–C ? phase would occur. Approaching this transition, R would be increasing, as would the susceptibility, χP , as seen in the ?gures above. The value of R could well remain sub-visible throughout the range of the modulated phase. The electroclinic e?ect could be large throughout the temperature range of the modulated phase, with a rapid increase as the transition to the helical Sm–C ? phase is approached. The mean smectic layer spacing would be almost constant through the phase transition. In the modulated phase it would be governed by an average between the layer spacing in the bulk and that in the side walls of the hexagonal cells, in which it is probably larger, due to a smaller molecular tilt angle. Therefore, at the phase transition, when the walls disappear, a very slight decrease in mean layer spacing would result. Qualitatively, these features agree with observations.

7

50

45

R
40

35

30 0.4 0.45 0.5

w
FIG. 5: The side R of the hexagonal unit cell determined by numerically solving Eq. (10), using Eq. (13), and choosing 2 K = 1, K ′ = AS = 0.1 and K2 q 2 + P0 /(8π?) = 0.0025.

0 -0.0005 -0.001 -0.0015

f
-0.002 -0.0025 -0.003 -0.0035 -0.004 0.4 0.45 0.5

w
FIG. 6: The approximate free energy density Eq. (14) as a function of w. The side R of the unit cell is determined numerically 2 from Eq. (10). The parameters used in Eqs. (10) and (5) are: K = K2 = 1, K ′ = AT = AS = 0.1 and K2 q 2 +P0 /(8π?) = 0.0025.

8

2500

χ

2000

1500

1000 0.4 0.45 0.5

w
FIG. 7: The susceptibility χP in arbitrary units as a function of w, determined from Eq. 15) and the numerical solution of Eq. 10).

One could try to orchestrate a more physically appealing model of how the parameters of the free energy might change with temperature. For instance, AS steadily increasing would have essentially the same result as w steadily 2 decreasing. More generally, any combination of K2 q 2 + P0 /(8π?) increasing and/or fW decreasing with falling temperature could produce the qualitative features of the apparent Sm–A phase and the phase transition. The most valuable test for the validity of this model in real materials would be the direct observation of the periodic structure of the modulated phase. The ?rst appropriate sub-optical probe that comes to mind is small angle X-ray di?raction, especially resonant X-ray di?raction that is most sensitive to variations of molecular orientation in a structure [10]. Hiroshi Yokoyama [11] has pointed out to us that atomic force microscopy might also be a suitable probe, if the modulated phase structure is preserved in a thin layer deposited on a substrate. Remarkably, in a recent paper [12] on one of the materials whose properties stimulated this work, optical observations consistent with a modulated phase, just at the transition from the Sm–A to the Sm–C ? phase, are reported. In a thin layer of material in the “bookshelf” geometry, i.e., the smectic layers viewed edge-on, thin parallel stripes are observed running perpendicular to the smectic layers. These stripes are possibly consistent with the long thin hexagonal cells that we propose here.
Acknowledgments

We thank R. Pindak for helpful discussions. This work was supported by the National Science Foundation under grants DMR–9873849 and DMR–9974388.

[1] For a recent review, see R. D. Kamien and J. V. Selinger, J. Phys.: Condens. Matter 13, R1 (2001). [2] S. Garo? and R. B. Meyer, Phys. Rev. Lett. 38, 848 (1977). [3] A. de Vries, A. Ekachai, and N. Spielberg, Mol. Cryst. Liq. Cryst. Lett. 49, 143 (1979); A. de Vries, Mol. Cryst. Liq. Cryst. Lett. 49, 179 (1979). [4] J. V. Selinger, P. J. Collings, and R. Shashidhar, Phys. Rev. E 64, 061705 (2001).

9
[5] [6] [7] [8] [9] [10] P. G. de Gennes and J. Prost, The Physics of Liquid Crystals (Clarendon Press, Oxford, 1993). S. A. Langer and J. P. Sethna, Phys. Rev. A 34, 5035 (1986). G. A. Hinshaw, R. G. Petschek, and R. A. Pelcovits, Phys. Rev. Lett. 60, 1864 (1988) G. A. Hinshaw and R. G. Petschek, Phys. Rev. A 39, 5914 (1989). E. Gorecka, M. Glogarov?, L. Lejˇek, and H. Svereny?k, Phys. Rev. Lett. 75, 4047 (1995). a c a L.S.Matkin, S.J.Watson, H.F.Gleeson, R.Pindak, J.Pitney, P.Barois, A.M.Levelut, G. Srajer and J.Pollmann., Phys. Rev. E 64, 21705 (2001), L.S.Matkin, H.F.Gleeson, P.Mach, C.C.Huang, R.Pindak, G.Srajer, J.Pollmann, J.W.Goodby, M.Hird, and A.Seed, Appl. Phys. Lett. 76, 1863 (2000). [11] Private communication. [12] A.Tang, D.Konovalov, J.Naciri, B.R.Ratna, and S.Sprunt, Phys. Rev. E 65, 010703(R) (2002).



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