The organization of nanoparticles in constrained geometries is an area of fundamental and practical importance. Spherical confinement of nanocolloids leads to new modes of packing, self-assembly, phase separation and relaxation of colloidal liquids; however, it remains an unexplored area of research for colloidal liquid crystals. Here we report the organization of cholesteric liquid crystal formed by nanorods in spherical droplets. For cholesteric suspensions of cellulose nanocrystals, with progressive confinement, we observe phase separation into a micrometer-size isotropic droplet core and a cholesteric shell formed by concentric nanocrystal layers. Further confinement results in a transition to a bipolar planar cholesteric morphology. The distribution of polymer, metal, carbon or metal oxide nanoparticles in the droplets is governed by the nanoparticle size and yields cholesteric droplets exhibiting fluorescence, plasmonic properties and magnetic actuation. This work advances our understanding of how the interplay of order, confinement and topological defects affects the morphology of soft matter.
Programmable organization of nanoparticles (NPs) in new structures is an important target of materials science and nanotechnology1,2,3. The organization of NPs in constrained geometries such as thin films or narrow channels is a valuable strategy for the generation of novel structures with potentially useful properties4,5,6,7,8. Spatial constraints can break the symmetry of confined structures and lead to a strong deviation from an equilibrium morphology. Confinement-mediated organization of particles in spherical space, e.g., in spherical droplets is of particular interest, since it offers the conditions of an isotropic confinement and controlled curvature for fundamental studies of particle packing9, self-assembly10,11 and relaxation of colloidal liquids12. Practically, phase separation of colloidal dispersions in spherical confinement can be used for the generation of multicomponent particles, for example, Janus particles13. Self-assembly of colloids in droplets paves the way for producing patchy structures mimicking atoms and molecules14.
Spherical confinement of liquid crystals formed by NPs offers a large parameter space for the generation of new structures. Macroscopic liquid crystals formed by viruses15,16 or carbon nanotubes17,18 have been reported; however, the organization of colloidal liquid crystals in spherical droplets remains a largely unexplored area of research, especially, for cholesteric (Ch) phases. Droplets of colloidal Ch liquid crystals can exhibit topological defects that can be used for fundamental studies of soft matter19,20 and as templates for the organization of molecules21 and NPs22,23. In comparison with molecular mesogens, the organization of NPs in liquid crystalline droplets adds a new set of length scales, thus making these droplets act as hosts for other types of NPs. Moreover, since the interplay of elastic and surface energies in droplets of thermotropic liquid crystals and the coupling of the properties of liquid crystals and NPs may yield structures with new optical and photonic properties24,25,26, these studies can be extended to colloidal lyotropic systems, especially, if their birefringence is enhanced by additives6, or by increasing NP volume fraction27.
Here we report the organization of rod-shape cellulose nanocrystals (CNCs) in Ch liquid crystals in the spherical confinement of micrometer-size droplets. In marked difference with droplets formed by thermotropic Ch mesogens28, confinement of the Ch–CNC liquid crystal results in phase separation into an isotropic phase in the droplet core and a Ch phase with concentric packing of the CNC layers at the droplet periphery. Further progressive confinement causes a transition to a bipolar planar Ch structure. For the droplets used as hosts for polymer, metal, carbon and metal oxide nanocolloids, we show the capability to control NP partition in the isotropic core and Ch shell and form Ch–CNC droplets with plasmonic, fluorescence and magnetic properties, respectively.
Spherical droplets of Ch colloidal liquid crystal
Figure 1a shows a transmission electron microscopy (TEM) image of negatively charged, rod-like CNCs with an average length L and diameter D of 183 and 23 nm, respectively. An aqueous 7 wt% CNC suspension, with a volume fraction of CNCs of 0.046, was equilibrated for 21 days. Following equilibration, the suspension phase separated into two co-existing phases (Fig. 1b), in agreement with earlier reports29,30, that is, into an isotropic top phase with the volume fraction of CNCs of 0.044 and a Ch bottom phase with the volume CNC fraction φ0=0.048. The volume fraction of the Ch phase in this two-phase system was 0.55 (Supplementary Fig. 1a). In the Ch phase, the CNCs exhibited long-range orientational order combined with their helical alignment. Polarized optical microscopy (POM) images of the Ch phase showed a multidomain mosaic pattern with characteristic stripes, with the axis of the Ch helicoid distorted in space (Supplementary Fig. 1b,c). The pitch of the Ch phase measured as a double distance between two adjacent stripes was P=6.0±0.3 μm.
The Ch phase was separated from the two-phase system and emulsified in a microfluidic flow-focusing droplet generator31. A fluorinated oil (F-oil) containing 1.0 wt% of a surfactant triblock copolymer perfluoropolyether and poly(ethylene oxide-co-propylene oxide) and the Ch phase were supplied to the microfluidic device as a continuous and droplet phases, respectively (Fig. 1c). In the orifice, the shear stress imposed by the two outer F-oil streams on the inner thread of the Ch phase resulted in a periodic breakup of the aqueous stream into uniformly sized droplets with a polydispersity of 2.5%. The droplet radius, R, was varied from 40 to 60 μm by changing the volumetric flow rate of F-oil from 1.5 to 0.3 ml h−1 at a constant flow rate of the Ch phase at 0.2 ml h−1.
Figure 1d–g shows the bright-field (BF) and the POM images of the droplets with a radius R=45 μm. The POM images showed the characteristic features of the Ch phase, that is, a Maltese cross and a shell with alternating bright and dark concentric rings corresponding to the surfaces of constant refractive index26 (a similar ring pattern is shown in the BF image in Fig. 1f). This structure of the droplet shell corresponded to the tangential CNC alignment at the droplet/F-oil interface with a radial orientation of the helical axis showing the direction along which the local orientation of the CNCs twists in space. The local orientation of the CNCs was described by the so-called director field . (Note that and were orthogonal to each other). The average pitch P in the Ch–CNC droplets, measured as a double distance between two adjacent concentric rings, was 6.1±0.3 μm, that is, close to P=6.0±0.3 μm of the macroscopic Ch phase. The central region of the droplets with a radius of 8.5±1.1 μm was formed by the isotropic phase. The equilibrium droplet structure was reached via transient states32. Spherical concentric packing of the Ch layers started at the droplet/F-oil interface, being assisted by the tangential surface anchoring of the CNCs, and with equilibration time, it gradually propagated toward the droplet centre (Supplementary Fig. 2).
Usually, confinement of rods between parallel planar substrates is expected to enhance the orientational order of the system33,34; however, spherical confinement of Ch phases leads to a different situation, in which the equilibrium state must be accompanied by a particular minimum number of defects, as dictated by topology. A Ch droplet with an infinitely strong tangential anchoring of the director at the droplet surface should acquire spherical packing of Ch pseudo-layers, which implies that the normal to these layers forms a radial point-defect hedgehog with the core in the droplet centre32. In such droplets, the director within each spherical pseudo-layer must contain defects, according to the Euler–Poincaré theorem32. When the spherical pseudo-layers are confined in a concentric manner within the Ch droplet, these point defects form radial defects—disclinations—in the local director field (ref. 32). Furthermore, if the equilibrium is not perfect, the Ch droplet may contain additional defects, such as dislocations that are associated with, for example, partial insertion or removal of the concentric layers.
Thus the equilibrium state of the Ch–CNC droplets with a tangential alignment of the director at the Ch/F-oil interface could not be realised without a point defect in the radial distribution of the normal , accompanied by the radial disclination lines in the director field . Near the equilibrium, dislocation defects were also possible.
The experimental results, in general, supported these expectations. In Fig. 1f,g, the point defect is evidenced by the concentric packing of the Ch–CNC pseudo-layers (which implies a radial configuration of the field ). The equilibrium disclination is marked with a white arrow, while an occasionally encountered dislocation is marked with a red arrow. The equilibrium disclinations were necessitated by the spherical confinement topology in the regime of strong chirality, when R>>P35,36. As demonstrated in the next section, this ideal structure expected on the basis of topological considerations was realised only partially, since the structure of the Ch–CNC droplets exhibited a strong dependence on their size.
Size dependence of the internal structure of Ch–CNC droplets
The effect of confinement on the droplet morphology was examined as a function of the droplet size for three cases.
Very-large drops with R>115 μm exhibited a multidomain Ch structure, similar to the macroscopic Ch–CNC phase (Supplementary Fig. 3). A multidomain morphology of large droplets with the axis of the Ch helicoid distorted in space was a manifestation of a very-long time needed for their complete equilibration. In this regard, the very-large droplets behaved similarly to the macroscopic Ch–CNC phase.
Inspection of droplets with a radius in the range 5≤R≤115 μm revealed that they had three types of ‘monodomain’ structures (Fig. 2a–c). The corresponding schematics of the CNC orientation in these droplets are shown in Fig. 2d–f, where the Ch layers are presented as surfaces separated by half-pitch. The distribution of the populations of droplets with different morphologies is shown in Fig. 2g.
For large droplets with dimensions in the range 40≤R≤115 μm (6.5≤R/P≤18.8), ∼96% of the droplets exhibited a Ch shell with a concentric packing of CNC pseudo-layers and thus radial configuration of the normal that formed a radial point-defect hedgehog. In these droplets, we observed either one radial disclination of strength 2 (Fig. 1g) or two radial disclinations of strength 1 each (Supplementary Fig. 4). In both cases, the total topological charge was two, equal to the Euler characteristic of the sphere, as required by the Euler–Poincaré theorem32. A single radial disclination was observed in ∼90% of the droplets, in agreement with numerical simulations and experimental observations of Ch droplets formed by thermotropic molecular liquid crystals28,37.
The most striking feature of the droplets with a concentric Ch layer packing was that the radial point defect exhibited an isotropic core with a radius, ri, in the range from ∼3 to 8.3 μm (∼0.5–1.4 P; Fig. 2a,d). The size of the core was larger in smaller droplets (Supplementary Fig. 5). With the droplet radius R decreasing from 115 to 40 μm, the volume fraction ∼ri3/R3 of the isotropic core in the droplet increased from 2 × 10−5 to 9 × 10−3 (Fig. 3a). This result suggested that spherical confinement caused phase separation in the system that exhibited a single-phase Ch behaviour in macroscopic samples, with the isotropic phase appearing at the core of the radial point defect. It was thus of interest to explore whether the same spherical confinement conditions would cause a change in the Ch pitch in the droplets. Fig. 3b shows the effect of the local curvature 1/Rloc on the pitch of the Ch shell, where Rloc was measured from POM images as the radial distance between the droplet centre and bright concentric rings in the Ch shell, starting from the second ring. For droplets with a radius of 45 and 100 μm, filled with the Ch phase at φ0=0.048, with the local curvature increasing from 0.01 to 0.08, the pitch remained invariant at P≈6.1 μm. On the other hand, similarly to the macroscopic Ch–CNC phase29, the Ch pitch in the droplets depended on the CNC concentration: when φ0 increased from 0.036 to 0.054, the pitch changed from 7.9 to 5.2 μm (Fig. 3c).
Intermediate-size droplets with 10≤R≤40 μm exhibited a transitional ‘ellipsoidal concentric layer’ pattern corresponding to planar Ch pseudo-layers in the centre and tangential CNC orientation at the droplet periphery (Fig. 2b,e). A large fraction of droplets with R≤20 μm (R/P≤3.3) displayed a stripe pattern characteristic of flattened Ch layers trapped between the two diametrically opposite poles (Fig. 2c). Notably, the interpretation of POM images for the intermediate-size droplets and for the small droplets with R≤10 μm (see below) depended on droplet orientation: when the axis of the Ch structure pointed up, a concentric ring structure was observed. Thus the morphology of these droplets was examined by carefully rotating them in the fluid cell (see, for example, Supplementary Movie 1).
Small droplets with R≤10 μm exhibited almost exclusively a bipolar stripe pattern. For such droplets, at φ0=0.048, the pitch remained invariant at 7.1 μm with increasing droplet size (Fig. 4a). When the droplets were formed from the Ch–CNC phase with varying φ0, the pitch showed the dependence on the volume fraction of the CNCs: an increase in φ0 from 0.036 to 0.054 resulted in the reduction of the pitch from 9.1 to 5.7 μm, respectively (Fig. 4b).
The transition from the ellipsoidal concentric layers to flattened Ch layers occurred at approximately Rtr≈10 μm. For the droplet size of Rtr, the elastic energy of spherical packing of the Ch-CNC layers that scales as KR, and the surface anchoring energy of the planar CNC layers that scales as WR2, were approximately equal to each other32. The balance of these two energies enabled the estimation of the surface anchoring strength, W, at the Ch droplet/F-oil interface, as W≈K/Rtr≈10−6 J m−2, where K is the average value of the Frank elastic constant that was assumed to be on the order of 10 pN (refs 38, 39), as for other lyotropic liquid crystals.
Distribution of nanocolloids in the Ch–CNC droplets
In assumption that the micrometer-size isotropic core in the Ch–CNC droplets can be used for the incorporation of chemicals or other nanocolloids, we loaded the droplets with spherical negatively charged 54 and 184 nm-diameter fluorescent dye-labelled polystyrene latex NPs and examined the effect of NP size on their distribution within the droplets. In equilibrium, a macroscopic mixture of the Ch–CNC phase and latex NPs phase separated into a latex-rich isotropic phase and a CNC-rich Ch phase (Supplementary Fig. 6 and Supplementary Note 1). The volume fraction of the isotropic phase increased at a higher volume fraction of latex NPs, φNP.
Droplets were generated in the microfluidic droplet generator immediately after mixing the Ch phase and latex NPs at φNP=0.0052 and subsequently, equilibrating droplets for 72 h. In the droplets, the NPs segregated in the cores of disclinations, similarly to the effect described for disclinations in thermotropic systems21,40,41 and in the isotropic core of the radial hedgehog (Supplementary Figs 7 and 8, respectively). The Ch shell structure of the droplets with a pitch P of ∼7 μm was preserved. The extent of partition in the droplet core increased with NP dimensions (Fig. 5a–h and Supplementary Fig. 9a–d). Examination of the variation of the ratio of the core-to-shell fluorescence intensities, based on the fluorescence microscopy (FM) images of the droplets revealed that ∼70 and ∼93% of 54 and 184 nm NPs, respectively, resided in the isotropic core of the hedgehog defect (Fig. 5j,k). Because of the stronger phase separation between the CNCs and the latex NPs with increasing latex content in the system, the extent of latex segregation in the isotropic core increased at higher φNP (Fig. 5k and Supplementary Figs 10–12), and the radius of the isotropic core increased from 12 to 30 μm (Fig. 5j and Supplementary Fig. 11). In contrast with small latex NPs, larger microspheres with a diameter of 1,000 nm formed multi-particle aggregates randomly distributed within the droplets (Fig. 6 and Supplementary Fig. 9e,f).
With the goal to extend the range of functionalities of the Ch–CNC droplets, we examined the organization of plasmonic gold NPs, fluorescent carbon NPs (carbon dots) and magnetic iron oxide rod-shape NPs, in the Ch–CNC droplets. In comparison with molecular Ch liquid crystals, a relatively large (∼30 nm (ref. 29)) average spacing between the CNCs in the Ch–CNC phase could accommodate small-size NPs. Droplets loaded with NPs were generated by the microfluidic emulsification of the Ch phase mixed with NPs. Figure 7a, top and bottom, shows transmission electron microscopy images of 10 and 50 nm gold NPs capped with thiol-terminated poly(ethylene glycol) with a molecular weight Mn=5,000 g mol−1. Small 10 nm gold NPs exhibited a uniform spatial distribution (Fig. 7b, top) in the core-shell Ch–CNC droplets, while 50 nm NPs partitioned in the isotropic droplet centre (Fig. 7b, bottom). Extinction spectra of the droplets loaded with gold NPs showed surface plasmon resonance a wavelengths similar to the corresponding bands of NPs in a macroscopic aqueous dispersion (Fig. 7c), indicating good NP dispersibility in the droplets and the capability to form plasmonic Ch–CNC droplets, with the NPs residing either in the Ch phase, or in the isotropic phase.
Droplets loaded with ∼3.5 nm-size fluorescent carbon dots (Fig. 7d) exhibited a uniform distribution in the Ch–CNC droplets, based on the distribution of fluorescence intensity within the droplets (Fig. 7e and Supplementary Fig. 13). The droplets exhibited a green emission colour when the NPs were excited at λexc=440 nm (Fig. 7f), while blue and red emission colours were obtained at λexc of 365 and 550 nm, respectively (Supplementary Fig. 14), due to the intrinsic excitation-dependent properties of carbon dots42.
In contrast with small gold NPs and carbon dots, magnetic Fe3O4/SiO2 rods with an average diameter and length of 100 nm and 1 μm, respectively (Fig. 8a), formed micrometer-size aggregates in the droplets (shown in Fig. 8b, top). This effect was consistent with the aggregation of large 1,000 nm latex microspheres in the Ch–CNC droplets. These aggregates moved towards a magnet placed outside the cell filled with the emulsion of the Ch–CNC droplets loaded with magnetic rods (Fig. 8b, bottom). Both translational motion of the droplets with acceleration of 1.7 μm s−2 (Fig. 8c and Supplementary Movie 2) and rotational droplet motion (Supplementary Movie 3) were achieved under the action of magnetic field.
The existence of a large isotropic spherical region in the Ch droplet centre (Fig. 2a) was in striking difference with enhanced order in nematic phases confined between planar surfaces33,34. We ascribe this difference to the spherical confinement of the Ch–CNC phase, which in equilibrium resulted in defects such as linear disclinations and the radial point-defect hedgehog. In contrast with a spherical confinement, an ideal flat confinement in equilibrium would not require any defects, nor isotropic inclusions, since the Ch phase separated at the binodal from its isotropic counterpart should reach a homogeneous structure at equilibrium.
Confinement by the spherical Ch/F-oil interface imposed spherical curvature of the Ch pseudo-layers, due to the finite surface anchoring that sets the helical axis perpendicular to the interface. To realign into a tangential orientation, one would need to perform the work against the anchoring energy that scales as WR2 (ref. 32). On the other hand, the energy of elastic distortions associated with the spherical curvature of pseudo-layers within the droplet scales as KR. Therefore, droplets with a large radius, R>K/W, would tend to preserve concentric spherical packing of the Ch pseudo-layers, while satisfying the boundary anchoring conditions, with being orthogonal to the Ch/F–oil interface. For R>K/W, the anchoring energy penalty is significantly larger than the elastic cost of the concentric packing, that is, WR2>>KR. Thus for the surface anchoring energy W=10−6 J m−2 and the elastic constant K=10 pN, droplets with a radius R larger than Rtr=K/W∼10 μm tend to curve the Ch layers and form concentric spherical layers, to preserve the surface anchoring conditions. On the other hand, when R<K/W, the structure with flattened layers is energetically preferred, that is, WR2<<KR.
The spherical packing of the Ch layers implies a radial configuration of the normal to the Ch layers, with the components written in the Cartesian coordinates. As one approaches the centre of the droplet at (x,y,z)=(0,0,0), the spatial gradients of and thus the elastic energy density strongly increase. Such an increase can be avoided if the regions with strong gradients adopt a less ordered structure, by e.g., local melting into an isotropic phase32. The effect of isotropic core has been considered in details theoretically for dislinations43 and for radial point defects hedgehogs44 formed in spherical volumes of a thermotropic nematic liquid crystal doped with a non-mesogenic additive. Analytical solutions are difficult, but the numerical simulations show that the isotropic core of the point defect can have a radius between 2 and 50 nm in pentylcyanobiphenyl (5CB), a typical thermotropic nematic liquid crystal44. Recent observations of defect loops with a 10 nm radius formed at the core of point defects in thermotropic liquid crystals support these predictions45. In our experiments, we attribute the appearance of a significantly larger core with a radius ri>1 μm, to the lyotropic nature of the liquid crystal system with the low concentration of the solute. Interestingly, large defect cores have been observed in another type of lyotropic liquid crystals, the so-called chromonics46.
To understand the mechanism of the appearance of the large isotropic core in the lyotropic Ch–CNC droplets with confinement-imposed spherical packing, we consider the balance of the elastic, condensation and surface energies associated with the cores, following the earlier models43,44,46,47. The free energy of the formation of an isotropic core with a radius ri in the centre of the Ch droplet with a radius R>>P and concentric packing of the Ch layers in the droplet shell is
where the first, the second and the third terms are the energy of elastic distortion of the Ch layers in the droplet shell, the surface energy of the Ch-isotropic interface, and the free energy difference between the isotropic and Ch phases, respectively. Here K1 and K24 are the splay and saddle-splay elastic constants of the Ch phase, respectively, σchi is the interfacial tension at the Ch-isotropic interface, and fi and fch are the free energy densities of the isotropic and Ch phases, respectively. In the coarse-grained model32 for the gradients of the field the (volume) free energy density is written as .
The first term in equation (1) is obtained by integrating the elastic energy density, fel given above, with and , over the Ch–CNC shell volume; here is the radius-vector of the spherical coordinate system, and r is the distance from the droplet centre32. Since K1—K24>0 (to ensure the flat configuration of the Ch layers of an unbounded system)32, σchi>0 and fi—fch>0, the term that favors the existence of the isotropic core is −8π(K1—K24)ri, by which the elastic energy is reduced when the highly curved Ch layers in the droplet centre are replaced with an isotropic spherical region. High elastic energy of distortions at the droplet centre is the main mechanism leading to the appearance of the isotropic core.
For a lyotropic system, an isotropic core implies that a fraction of CNCs is transferred from the core into the Ch shell. Therefore, equation (1) should be supplemented by the mass conservation law44
where φi and φch are the CNC volume fractions in the isotropic and Ch regions of the droplet. For the studied range of radii of the Ch–CNC droplets, the volume fraction φch of the CNC in the Ch shell does not significantly differ from the CNC volume fraction φ0 of the emulsified single-phase macroscopic Ch–CNC phase. For example, even if all the CNCs were expelled from the isotropic core, for (ri/R)3 as large as 9 × 10−3 (which is the case of droplets with R=40 μm) the volume fraction of CNC in the shell, φch=0.0481 would be only a little higher than the initial volume fraction of CNCs φ0=0.048. The difference φch−φ0 becomes even smaller as the droplet radius increases. The small difference between φch and φ0 explains why the Ch pitch measured in the shells of the biphasic Ch–CNC droplets is almost the same as in the macroscopic Ch phase.
The system of equations (1) and (2) can be solved only numerically44, however even a numerical treatment is problematic, since the thermodynamic characteristics of the system under study are not known. To obtain an order of magnitude estimate of the isotropic core radius, we approximate the free energy density difference in equation (1) through the chemical potentials of the isotropic (μi) and Ch (μch) phases (Supplementary Note 2), as fi−fch≈(μi−μch)/vCNC, where vCNC is the volume of an individual CNC (Supplementary Methods). Furthermore, the difference between the chemical potentials can be estimated on the ground of translational-orientational entropy differences between the isotropic and Ch phases as μi−μch≈αkBTφ0b/vCNC≈αkBTφ0L/D. Here α is the numerical parameter of the order of 1, which depends on the exact shape and size distribution of CNCs, kB is the Boltzmann constant, T is the absolute temperature, and b=πL2D/4 is the average excluded volume of a CNC with a length L and diameter D. In what follows, we denote (μi−μch)/vCNC≈4αkBTφ0/(πD3) as Δf. To obtain an estimate for the equilibrium radius ri* of the isotropic core, we assume that the interfacial tension σchi and Δf do not depend on the droplet size. By minimizing the energy in equation (1) with respect to ri, one finds
The interfacial tension σchi between the isotropic and Ch phase formed by aqueous CNC suspensions is in the range of 10−7−10−6 J m−2, as determined experimentally48. The value of Δf defined above, for α=1, is estimated to be 20 J m−3. For K∼10 pN (refs 38, 39), as for other lyotropic liquid crystals, equation (3) predicts an equilibrium radius ri* to be on the order of 1 μm, which is close to the experimentally measured core size. Note that for vanishingly small Δf, the equilibrium radius would be ri*=(K1−K24)/σchi, thus potentially achieving the value in the range 10–100 μm.
This relatively large, 1 μm or more, core radius is by two or even three orders of magnitude larger than a 10 nm core size of point defects in thermotropic liquid crystals44,45.The reason for the large core is that the quantity Δf estimated above is significantly smaller than the corresponding latent heat of the isotropic–nematic transition in thermotropic liquid crystals. For typical thermotropic liquid crystals, for example, 5CB, the latent heat is on the order of 106 J m−3 (refs 32, 49), that is, five orders of magnitude higher than Δf in the Ch–CNC phase.
The reorganization from concentric to flattened packing of the Ch layers (Fig. 2) observed at decreasing R/P ratio and caused by the finite surface anchoring at the droplet/F–oil interface was in qualitative agreement with earlier numerical simulations28 and experimental results37 for thermotropic Ch droplets. We ascribe this structural transition to the balance between the surface energy of the droplets (that scales as WR2) and the elastic energy of Ch deformations (that scales linearly with the radius, as KR)32. In large droplets (Fig. 2a), the surface anchoring of CNCs led to concentric packing of strongly curved layers, which remained parallel to the droplet surface, while in small droplets (Fig. 2c), the layers flattened at the expense of partial violation of boundary conditions. Tangential anchoring of the director at the Ch/F–oil interface acted to unwind the Ch helix, thus enlarging the Ch pitch, as observed experimentally.
The collective behaviour of colloid particles in the Ch–CNC droplets was governed by the NP size. Earlier studies of phase separation in mixtures of rods and spheres16,50,51,52,53, as well as the discussion above on the appearance of the isotropic central core, suggest that phase separation of NPs in the Ch–CNC phase should be expected. The 54 and 184 nm latex NPs fit into the cores of defects and thus gained a freedom of translational motion within an isotropic phase. In the Ch shell, smaller 54 nm NPs were less disruptive to the Ch structure than larger 184 nm NPs, since the average distance between the CNCs is about 30 nm (ref. 29). Placement of 184 nm NPs into a Ch shell was apparently energetically more costly, as these NPs could distort the director. To calculate the actual energy cost of placing the NPs in the isotropic and Ch parts of the droplets more information is needed on surface interactions. The increase in the radius of the latex-rich isotropic cores with increasing φNP stemmed from the stronger phase separation between the latex-rich isotropic phase and the CNC-rich Ch phase, as shown for the macroscopic mixture of the Ch–CNC phase and latex NPs (Supplementary Fig. 6c and Supplementary Note 1).
Larger 1,000 nm-diameter latex beads and 1,000 nm-long magnetic nanorods were observed in both the Ch shells and in the isotropic cores. The plausible reason is that these large particles are kinetically trapped in out-of-equilibrium states during the sample preparation, when the Ch–CNC phase was mixed with the NPs. Large particles perturbed the Ch director around them and attracted each other through long-range elastic forces50,54,55,56. If the surface anchoring at the NP–Ch interface is strong, the typical order of magnitude of the elastic energy of interaction is ∼Kd, where d is the size of the colloid particle. When d is 1 μm, the elastic energy of interaction can reach ∼10−17 J, that is, orders of magnitude higher than the thermal energy, 4 × 10−21 J. Therefore, large particles can form kinetically trapped clusters with irregular shapes that cannot relax into equilibrium shapes, due to very large (compared with thermal energy) energy barriers. A similar behaviour and physical mechanism have been described for the thermotropic Ch phase doped with 1 μm silica particles, which formed irregular clusters and were not responsive to thermal annealing57.
Finally, our experiments show that the smallest 3.5 nm carbon dots and 10 nm gold NPs do not exhibit partitioning between different regions of the Ch droplets. These particles could fit between the CNCs and did not perturb the Ch structure.
In conclusion, progressive spherical confinement of Ch phases formed by rod-shape CNC colloids resulted in new structures and transitions between them. Notably, confinement-induced phase separation of the Ch–CNC phase enabled a single-step preparation of core-shell droplets with a controllable Ch shell thickness, a method that is simpler than current methods for the preparation of liquid crystalline shells58,59. These structures can be used in fundamental studies of defects in frustrated liquid crystalline phases60, and for the engineering of particles with unusual mechanical and structural properties61,62. There is also a potential for optical applications of the droplets, since on evaporation of water from the Ch–CNC phase, the pitch is reduced and the resulting material selectively reflects light in the visible spectral range30. In aqueous suspensions, birefringence of CNCs normalized by their volume fraction is ∼0.12 (ref. 27). For the volume fractions of CNCs used in our experiments, the effective birefringence (calculated for quasi-nematic regions of size significantly smaller than the pitch) is rather low, ∼0.006, however, it can be increased by adding special ingredients such as gold nanorods6 or by increasing the volume fraction of CNCs27.
The co-assembly of CNCs with polymer and inorganic NPs provides a route for the design of new stimulus-responsive liquid crystalline materials. Previously, topological defects have been used as templates for the organization of colloid particles and molecules in thermotropic liquid crystals, which are mostly hydrophobic materials21,41,45,63,64,65,66. Our results demonstrate that the topological defect (droplet core) in a hydrophilic medium, such as an aqueous CNC suspension, can also be used for NP organization. The plasmonic, fluorescent and magnetic properties of the NP-loaded Ch–CNC droplets broaden the range of potential applications which remain to be explored.
Generation and characterization of CNC droplets
The experimental details of the synthesis of NPs and the fabrication of microfluidic devices are given in the Supplementary Information (Supplementary Methods). The Ch–CNC droplets were produced by the emulsification of the aqueous Ch–CNC phase in the flow-focusing microfluidic droplet generator31. The Ch phase (Supplementary Methods) was injected as a droplet phase at a flow rate of at 0.2 ml h−1 into the central channel of the microfluidic device using a syringe pump (PhD 200 Harvard Apparatus PHD 2000 Syringe Pump, USA). The continuous phase (fluorinated oil HFE-7500 or F-oil) mixed with 1 wt% of the copolymer surfactant perfluoropolyether and poly(ethylene oxide-co-propylene oxide) was injected into the side channels of the microfluidic device using the second syringe pump (PhD 200 Harvard Apparatus PHD 2000 Syringe Pump, USA) at a flow rate varying in the range from 0.3 to 1.5 ml h−1. The Ch–CNC droplets exiting the microfluidic device were collected in a 2 ml glass vial and transferred into a cell consisting of two parallel glass slides separated by a 400 μm-thick spacer. The cell was sealed with epoxy glue and the droplets were equilibrated for various time intervals.
To prepare Ch–CNC droplets with a broad size distribution and radii up to 115 μm, a mixture of 200 μl of the Ch–CNC phase and 1 ml of F-oil was shaken at 50 Hz for 1 min at room temperature in a vortex mixer. For the preparation of droplets with dimensions up to 250 μm, a mixture of 200 μl of Ch–CNC phase and 1 ml F-oil containing 1 wt% of the copolymer surfactant was shaken at 30 Hz for 15 s at room temperature in a vortex mixer. The resultant emulsion of Ch–CNC droplets was introduced in the cell, the cell was sealed with epoxy glue and the droplets were allowed to equilibrate for 7 days.
The BF and POM imaging, and the video recording of the Ch–CNC droplets were carried out on an optical microscope (Olympus BX51) in the transmission mode. The diameters of the droplets and isotropic cores and the pitch of the Ch phase in the droplets were measured using the software ImageJ. The diameter of the isotropic droplet core was defined as the diameter of the innermost circle ring in the droplets, based on the BF images.
Generation and characterization of droplets loaded with NPs
The Ch–CNC droplets loaded with NPs were prepared by emulsifying a mixture of the Ch–CNC phase and NPs in the flow-focusing microfluidic device. The procedure was identical to that used for the preparation of NP-free Ch–CNC droplets. A mixture of 60 μl of the suspension of FITC-labelled latex NPs, carbon dots, gold NPs or magnetic nanorods and 540 μl of the Ch–CNC phase was prepared by shaking at 50 Hz for 2 min at 25 °C in a vortex mixer and immediately emulsifying this mixture in the microfluidic device.
The hybrid droplets were imaged using an optical microscope (Olympus BX51). The fluorescence images of the Ch–CNC droplets loaded with FITC-labelled latex NPs and carbon dots were acquired on an inverted microscope (Nikon Eclipse-Ti). The fluorescence intensity profiles of these droplets were measured using a software (NIS-Elements AR Analysis). The Z-stack fluorescence images of the Ch–CNC droplets loaded with FITC-labelled latex NPs and carbon dots were taken by Nikon A1 confocal microscope. The extinction spectra of the solution of gold NPs were acquired using Cary-5000 spectrophotometer. The extinction spectra of the emulsion of the Ch–CNC droplets loaded with gold NPs were acquired using a plate reader (CLARIOstar, Mandel) by placing the emulsion of Ch–CNC droplets in a 96-well plate. The photoluminescence of individual Ch–CNC droplets loaded with carbon dots was measured by using a LabRam-HR (JY Horriba). The confocal spectrometer was attached to a microscope to focus on the targeted areas of the droplet. The photoluminescence was excited at λexc=444 nm. The videos of translational and rotational movement of the Ch–CNC droplets loaded with magnetic nanorods were taken on an inverted microscope (Nikon Eclipse-Ti). Droplet displacement was measured by a software (NIS-Elements AR Analysis).
The authors declare that the data supporting the findings of this study are available within the article and its Supplementary Information Files, and all relevant data are available from the authors.
How to cite this article: Li, Y. et al. Colloidal cholesteric liquid crystal in spherical confinement. Nat. Commun. 7:12520 doi: 10.1038/ncomms12520 (2016).
We thank Connaught Foundation and NSERC Canada (Discovery and Strategic grants) for financial support of this work. E.K. is grateful to the Canada Research Chair programs (NSERC CANADA). O.L. acknowledges financial support from NSF DMR-1121288 and NSF DMS-1434185. B.Y. acknowledges financial support from The National Science Foundation of China (NSFC) under Grant No. 51373065. Y.L. acknowledges Banting Postdoctoral Fellowships program, administered by the Government of Canada and the International Postdoctoral Exchange Fellowship Program 2013 funded by the Office of China Postdoctoral Council (20130035). We are grateful to Professor Michael Rubinstein (The University of North Carolina) and Dr Oleg Gang (Brookhaven National Laboratory) for fruitful discussions. The authors thank Xiguang Gao for initiating preliminary experiments and Ilya Gourevich for assistance in imaging experiments.
About this article
Scientific Reports (2017)