The geometrical presentation of the generator of the full braid group for R2 and its inverse (left); in 2D (right).

3.2. Cyclotron Structure of Braid Group in 2D Charged Systems at Strong Magnetic Field Presence

The full braid group contains all accessible closed multi-particle classical trajectories, i.e., braids (with initial and final orderings of particles that may differ by permutation as is admitted for indistinguishable particles). One can, however, notice that inclusion of a strong magnetic field may substantially change trajectories―a classical cyclotron motion may confine a variety of accessible braids if magnetic field is strong enough and the manifold is two-dimensional. When the separation of particles is greater than twice the cyclotron radius, which situation occurs at fractional LLL fillings, the exchanges of particles along single-looped cyclotron trajectories are precluded, because the cyclotron orbits are too short for particle interchanges in this case. Interaction cannot enhance cyclotron orbit size in the uniform multiparticle system.

Particles must, however, interchange in the braid picture for the reason of defining the statistics and creation of the collective correlated state. Therefore, in order to allow exchanges again, the cyclotron radius must somehow be enhanced. This can be achieved by screening the external field, like in the construction of the CFs with flux tubes oppositely oriented with respect to the external field [22] . We suppose that the natural way to enhance the range of cyclotronic movement is to exclude inaccessible braids from the full braid group. We will show that remaining braids would be sufficiently large in size for particle exchanges realization [13] [14] . We will demonstrate below that at high magnetic fields in 2D charged N-particle systems, the multi-looped braids allow for the effective enlargement of cyclotron orbits, thus restoring particle exchanges in a natural way.

4. Cyclotron Braid Subgroups―Restitution of Particle Interchanges in 2D

The multi-looped braids form the cyclotron braid subgroups which are generated by the following generators:

, (3)

where each q corresponds to a different type of the cyclotron subgroup and are the generators of the full

braid group. The group element represents the interchanges of the ith and (i + 1)th particles with

loops, which is clear by virtue of the definition of the single interchange (cf. Figure 3, e.g., for q = 3 one

Figure 3. The generator σi of the full braid group and the corresponding relative trajectory of the ith and (i + 1)th particles exchange (upper); the generator of the cyclotron braid subgroup, (in the figure, q = 3), corresponds to additional loops when the ith particle interchanges with the (i + 1)th one (lower) (2R0 is the inter-particle separation, Rc is the cyclotron radius, 3D view added for better visualization).

deals with elementary particle exchange braid with one additional loop). It is clear that generate a subgroup of the full braid group as they are expressed by the full braid group generators.

The 1DURs of the full group confined to the cyclotron subgroup (they do not depend on i as 1DURs of the full braid group do not depend on i by virtue of the generators property, , , [11] ) are 1DURs of the cyclotron subgroup:

, (4)

where q is an odd integer and. We argue, that these 1DURs, enumerated by the pairs, describe composite anyons (CFs, for). Thus in order to distinguish various types of composite particles one has to consider 1DURs of cyclotron braid subgroups.

In agreement with the general rules of quantization [25] , the N-particle wave function must transform according to the 1DUR of an appropriate element of the braid group, when the particles traverse, in classical terms, a closed loop in the configuration space corresponding to this particular braid element. In this way the wave function acquires an appropriate phase shift due to particle interchanges (i.e., due to exchanges of its positions as arguments of the wave function, according to the prescription given by braids in 2D configuration space). Using 1DURs as given by (4), the Aharonov-Bohm phase of CFs fictitious fluxes is replaced by the contribution of additional loops (each loop adds 2π to the total phase shift, if one considers 1DUR with related to CFs, cf. Figure 3 (right)). Let us emphasize that the real particles do not traverse the braid trajectories, as quantum particles do not have any trajectories, but the exchanges of arguments of the N-particle wave function can be represented by braid group elements; in 2D an exchange of particle positions described by coordinates on the plane does not resolve itself to the permutation only, as it was in 3D, but must be performed according to an appropriate element of the braid group, being in 2D not the same as the permutation group [25] . Hence, for the braid cyclotron subgroup generated by, , we obtain the statistics phase shifts qπ for CFs (i.e., for in Equation (4)), as required by Laughlin correlations, without the need to model them with the auxiliary field flux tubes.

Each additional loop of a relative trajectory for the particle pair interchange (as defined by the generators) reproduces an additional loop in the individual cyclotron trajectories for both interchanging particles―cf. Figure 4. The cyclotron trajectories are repeated in the relative trajectory (c, d) with twice the radius of the individual particle trajectories (a, b). In quantum language, with regards to classical multi-looped cyclotron trajecto-

ries, one can conclude only about the number, , of flux quanta per single particle in the system, which for the filling is q (for odd integer q), i.e., the same as the number of individual particle cyclotron loops (which equals to, where indicates the number of additional braid-loops for particle interchange trajectories). From this observation it follows a simple rule: for (q odd), each additional loop

of a cyclotron braid corresponding to particle interchange, results in two additional flux quanta piercing the individual particle cyclotron trajectories. This rule follows immediately from the definition of the cyclotron trajectory, which must be a closed individual particle trajectory related to a double interchange of the particle pair (cf. Figure 5). In this way, the cyclotron trajectories of both interchanging particles are closed, just like the closed relative trajectory for the double interchange (the braid trajectory for the elementary exchange of the indistinguishable particles is open in the geometrical presentation, and therefore the double interchange is needed to close this trajectory in this presentation). If the interchange is simple, i.e., without any additional loops, the corresponding individual particle cyclotron trajectories are also simple, i.e., single-looped. Nevertheless, when the interchange of particles is multi-looped, as associated with the q-type cyclotron subgroup, the

double interchange relative trajectory has closed loops, and the individual cyclotron trajectories are also multi-looped, with q loops [14] .

In 2D additional loops cannot enhance the total surface of the system. In this regard, it is important to emphasize the basic difference between the circumvolutions of a 3D winding (e.g., of a wire) and of multi-looped 2D cyclotron trajectories. 2D multi-looped trajectories do not enhance the surface of the system and therefore do

Figure 4. Half of the individual particle cyclotron trajectories of the ith and (i + 1)th particles (top) and the corresponding relative trajectories (bottom) for interchanges of the ith and (i + 1)th 2D-particles under a strong magnetic field, for (left) and for (right), respectively (Rc―cyclotron radius, 2R0―particle separation, 3D added for better visualization).

Figure 5. Cyclotron trajectories of individual particles must be closed, therefore they correspond to double exchange braids, for both, simple exchanges (upper) and exchanges with additional loops (lower), in the right part, quantization of flux per particle, for and, is indicated.

not enhance the total magnetic field flux BS piercing the system, in opposition to 3D case. In 3D case, each circumvolution of the winding adds a new portion of the flux, just as a new circumvolution adds a new surface, which is, however, impossible in 2D. Thus in 2D all loops must share the same total flux, which results in diminishing flux-portion per a single loop and, effectively, in longer cyclotron radius (allowing again particle interchanges).

The additional loops in 2D take away the flux-portions (equal to flux quanta just at, q odd) si-

multaneously diminishing the effective field; this gives an explanation for Jain’s auxiliary fluxes screening the external field B. Thus, it is clear that the CFs are actually not compositions of particles with flux-tubes, but are rightful particles in 2D corresponding to 1DURs of the cyclotron subgroups instead of the full braid group, which is unavoidably forced by too short ordinary single-looped cyclotron trajectories. The original name “composite fermions” can be, however, still used for history reason. Moreover, one can use a similar name, “composite anyons”, for particles associated with fractional 1DURs (i.e., with fractional) of the cyclotron subgroup instead of the full braid group, the latter linked rather with ordinary anyons (without magnetic field).

How Additional Loops Enhance the Cyclotron Radius in 2D Hall System

It is important to emphasize that braid group approach in terms of trajectories does not describe detailed classical trajectories of particles in the system but only determines classes of trajectories which are available upon topological constraints. Thus, if one considers physical factors which restrict availability of particular classes of trajectories (e.g., specific topology of configuration space of N particles system located on specified manifold), one should describe a condition upon which one can determine whether a specific trajectory class is possible or not. In the case of N particles system on 2D plane in the presence of a perpendicular strong magnetic field such a condition can be based on the cyclotron radius. Although cyclotron radius is properly defined for free particles one can still consider some kind of focusing of charged particle motion on the cyclotron radius scale even in the presence of interaction, especially in homogeneous planar system with isotropic interaction. One can also observe that for noninteracting fermions we have in the case of completely filled LLL exactly one external field

flux quantum per particle which means that the cyclotron radius is defined by the single flux quantum.

Here must be emphasized that in the case of the degenerated LLL all particles have the same cyclotron radius. Even though the velocity is not well determined in the LLL (their coordinates do not commute as the operators), all particles have, however, the same kinetic energy, thus all particles have the same averaged velocity and the same cyclotron radius. In order to determine whether a trajectory class is available for particles in the system can be brought to comparison of cyclotron orbit size with distance between particles, which for homogeneous system is defined from density and blocked by Coulomb repulsion preventing approaching one particle onto another one. The distance between particles in homogeneous system is protected by the short-range part of the Coulomb interaction. Thus potentially available trajectory must ensure reaching neighboring particles, i.e., the trajectory must fit to the minimal distance between particles. The rigorous requirement to keep minimal distance intact leads to the observation that in too strong magnetic field (when the cyclotron radius is smaller than half of the minimal distance) some trajectory classes are unavailable for particles―as shown in Figure 6.

In 2D charged system in the presence of the perpendicular magnetic field only cyclotron trajectories are available for particles. Thus if one increases the magnetic field magnitude then the cyclotron radius will decrease causing the trajectory of particles exchange impossible. The simplest exchange was the implementation

Figure 6. Schematic presentation of effective growth of cyclotron radius in 2D case for multi-looped cyclotron trajectory in comparison to single-looped trajectory (length A − B means uniform separation between particles in the system).

of the generators of the full braid group and now they cannot be defined. If one excludes unavailable trajectories too short for exchanges, the rest of the full braid group occurs a subgroup generated by new generators describing in 2D multi-looped braids and corresponding to multi-looped cyclotron trajectories. These multi-looped cyclotron trajectories have the larger effective size allowing to match neighboring particles at strong magnetic field presence. This subgroup we call cyclotron braid group (or subgroup).

The exchange trajectories of neighboring particles―the generators of braid group―are open trajectories i the geometrical presentation (in fact for indistinguishable particles the initial and final particle ordering are bound despite remunerations, but for geometrical presentation of braid group some selected, arbitrary ordering of particles is assumed). Nevertheless, the cyclotron trajectories are closed trajectories despite the enumeration of particles (only for closed trajectories one can define the piercing flux of the magnetic field). Thus, one must consider closed cyclotron trajectories. The smallest closed trajectory is a double exchange (two semicircles create closed circle in the simplest case of single-looped exchanges). If now one considers multi-looped exchanges (for, q―odd), one has to take also into account closed trajectories related to cyclotron trajectories―each particle traverses a closed cyclotron trajectory with additional loops. Closed loops can be added only by one, therefore the simplest exchange with one additional loop results in three-looped cyclotron trajectory of individual particles. This explains why FQHE manifests in simplest case for. Summarizing this argumentation, we emphasize that additional loops can be added to single exchange trajectory (braid group generator) one by one (in order to keep the exchange character of the trajectory). Then to the closed trajectories (double exchange) must be added the double number of the additional loops, two in the case of. That is why braid trajectories are odd-looped trajectories (1, 3, 5, 7, etc. for respectively, , etc.) and not even-looped closed trajectories (such trajectories divided on half will not give an exchange trajectory). For LLL fillings particles traverse the closed individual cyclotron trajectories with additional loops and simultaneously open exchange trajectories with additional loops.

Those multi-looped closed trajectories in case of 2D have enhanced effective cyclotron radius which allows particles to exchange and to define the statistics. Each additional loop cannot add any new surface in 2D space. For e.g., the cyclotron radius is too short for exchanges. For each particle at corresponding magnetic field we have 3 flux quanta. But the cyclotron trajectory is defined by a single flux quantum. However, if one considers 3-looped cyclotron trajectory in 2D with the size as trajectory corresponding to then the total flux of external field does not change. The surface of the multi-looped trajectory also fits to the particle separation distance, but through every loop passes only single flux quantum because in 2D the total flux must be shared between all loops, which means that in the multi-looped case the effective cyclotron radius is greater than for single-looped trajectory. It is illustrated in Figure 6 for case and the arrow represents the single flux quantum defining the cyclotron radius.

The Coulomb interaction plays a central role in the collective state with Laughlin correlations [17] -[19] protecting the uniform equidistant distribution of particles. Nevertheless, in 2D systems upon the quantized magnetic field, the interaction of charges cannot be accounted for in a manner of the standard dressing of particles with the interaction as it was typical for quasiparticles in solids, because in 2D Hall regime this interaction does not have a continuous spectrum with respect to particle separation expressed by relative angular momentum projection [17] [18] . This non-continuous character of the interaction contribution in 2D charged systems upon sufficiently strong magnetic fields precludes the continuity of the mass operator which prevents the quasiparticle definition (as a pole of the retarded single-particle Green function).

5. Topological Chern Insulators

Investigation of IQHE and then of FQHE in 2D charged systems opened a broad area of topologically conditioned effects [26] . Especially deeply developed with this regard is the present understanding of IQHE treated in single-particle and topological terms [7] . This is based on the observation that the IQHE states protected by Landau quantization gaps are not connected with symmetry breaking as many other condensed matter phases in scenario of ordinary phase transitions, but rather with some topological invariants associated to a particular geometry and matter organization [6] [27] . These invariants are better and better recognized currently in terms of homotopy groups related to specially defined multidimensional transformations of physically conditioned objects like Green functions and their derivatives [28] [29] , previously developed for description of topology of textures in multicomponent condensed matter states with rich matrix order parameter, including superfluid He3 or liquid crystals [4] . The role of various factors protecting gaps separating flat bands (almost degenerated, as LLs at the interaction presence, and massively degenerated in the absence of the interaction) are of particular interest in view of the role of the magnetic field breaking time reversion or other effects like spin-orbit interaction or special type (time-reversion breaking) traversing around the closed loop inside an elementary cell with complex hopping constants. Generalization of the familiar in mathematics Chern invariants [5] is developed in order to grasp the essential topology of various multiparticle structures [5] -[7] . The mappings of the Brillouin zone into the state related objects can be in that manner classified by disjoint classes corresponding to topologically nonequivalent band organizations protected by energy gaps conditioned by various physical factors and leading to distinct incompressible states in analogy to their prototype in the form of IQHE. The distinctive character of 2D space is linked in the latter case with the magnetic field flux quantization.

Topological notions allow for definition of a new state of crystal called topological insulator. Despite of the local similarity between the gapped states of the ordinary and the topological insulator, the global arrangement of the band, noticeable only non-locally (on the Brillouin zone as a whole), induces different overall behavior of the system. In the case of topological insulator one deals with insulating state inside the sample, whereas with conducting non-dissipative state on the sample edge, protected topologically, what is, however, no case for ordinary insulating state. This surprising phenomenon was confirmed experimentally, which was a strong stimulus to the rapid and enormous great growth of the interest.

The topological insulators from point of view of band organization must be characterized by flat bands which meet in summits of locally cone shaped valleys resembling Dirac points in graphene. These Dirac points changes the topology and allow Chern-type invariant to attain nonzero value, indicating the emergence of the different global state. Spin degrees of freedom are of high significance with regard to topological arrangement and related spin-type topological insulators are referred as to spin IQHE.

Commonly accepted definition of the topological insulator emphasizes the robust metallic character of the edge or surface states and extended bulk insulating states that are also robust against disorder. This is an extraordinary behavior, especially in two-dimensional models―when an edge or a surface is cut in a sample of topological insulator, the emerging edge states seem to be connected to these bulk states. The edge states can be viewed as these extended bulk states terminating at the boundary. For this reason, the bulk and the edge properties of the topological insulators are equally important and mutually dependent. This is the development of the interpretation of IQHE revealed a spectacular emergence of non-dissipative charge currents flowing around the edges of any finite IQHE sample. The IQHE was observed only in the presence of an externally applied magnetic field.

In 1988 Haldane presented a model of a condensed matter phase that exhibits IQHE without the need of a macroscopic magnetic field [30] . The general idea of this effect can be sketched by writing a model Hamiltonian, for the system of spinless particles occupying a honeycomb-type planar lattice with one state per site,

, (5)

where indicates summation over nearest neighbors, whereas the symbol indicates that the summation includes also next-nearest neighbors, the hopping factor is assumed artificially as a complex number, and depending on how n is positioned in the unit cell (equivalently an isospin can be introduced here), as is shown in Figure 7. The essence of the topological effect is linked with imaginary contribution to hopping factor given by η. The band structure corresponding to this Hamiltonian depends on parameters t, η and exhibits nontrivial topological properties (expressed by the Chern number C) for various values t, η.

The difference between a quantum Hall state and an ordinary insulator is a matter of topology [8] . A 2D band structure consists of a mapping from the momentum k defined on a torus of the Brillouin zone to the Bloch Hamiltonian. Gapped band structures can be classified topologically by considering the equivalence classes of this mapping that can not be continuously deformed into one another without closing the energy gap. These classes are distinguished by integer topological invariants―the Chern numbers. The Chern numbers were introduced in the theory of fiber bundles [10] , and they can be understood physically in terms of the Berry phase [9] associated with the Bloch wave functions. When k traverses a closed loop, the Bloch function acquires a Berry phase given by the line integral of, or by a surface integral of the Berry field. The Chern invariant is the total Berry field flux for the Brillouin zone,

Figure 7. The honeycomb structure (similar as in graphene) for the Haldane model [30] ; e1, e2 are Bravais lattice vectors, nonequivalent site positions in the unit cell are indicated by.

, (6)

C is integer for reasons analogous to the quantization of the Dirac magnetic monopole. The Chern number, C, is a topological invariant in the sense that it cannot change when the Hamiltonian varies smoothly and this explains the quantization of conductivity in IQHE [8] . Helpful would be here a simple analogy. Rather than maps from the Brillouin zone to a Hilbert space, one can consider maps from two to three dimensions, which describe surfaces. 2D surfaces can be topologically classified by their genus g, which counts the number of holes. For instance, a sphere has g = 0, while a torus has g = 1. A theorem in mathematics states that the integral of the Gaussian curvature over a closed surface is a quantized topological invariant, and its value is related to g. The Chern number is an integral of a related curvature.

Change of the Chern number requires closing the insulating gap. This happens for the Hamiltonian (5) in the Dirac-like points when the locally cone shaped valleys of conduction and valence bands touch together. This allows for the change of the Chern number and for the metallic boundary states protected by still insulating phase inside the sample [6] [7] .

The systems that behave like the one described by Haldane are now called Chern insulators. The time reversal symmetry in these systems is broken like in the IQHE, but it is broken by the presence of a net magnetic moment in each unit cell rather than by an external magnetic field, as it was the case for IQHE. The Chern insulators were never found experimentally as of yet.

Fractional Chern Insulators

Recently grew up a new field related to IQHE and its fractional version, namely Chern insulators and fractional Chern insulators, respectively. There is linked with development of Haldane model of IQHE effect without Landau levels, but with time-braking imaginary part of hopping factors for carries on planar lattice instead of the external magnetic field. The quantization of carrier orbit along elementary cell is given in this case by the quantization of the Berry field flux which can be expressed by the Chern numbers. Even though neither Chern insulator nor its fractional state is not observed experimentally, the theoretical studies are currently extensively developing [31] [32] . From exact diagonalization of corresponding Hamiltonians, provided they give sufficiently flat bends, it follows that the interaction causes collective state analogous to FQHE, though without any magnetic field and with the dynamics assigned by nontrivial Chern number. What is especially challenging, the frac-

tional Chern insulator is predicted for fractional (, p―odd integer) fillings of planar crystal lattice, analo-

gously to ordinary FQHE. Again arises a question of how single particle trajectories ranged by Berry field flux quantization to the elementary cell can match every third cell (for 1/3 filling). The concept of CFs with auxiliary field flux-tubes is not useful here, due to absence of the magnetic field. The trajectories must be, however, enlarged somehow to allow organization of the collective state with the determined statistics via particle interchanges.

Again here the multi-looped braid subgroup might be the solution of the problem with too short orbits, especially in this case which is without any other conceptual competition (composite fermions are associated with magnetic field flux tubes, but here no magnetic field presents). This supports the topological attitude to fractional correlated 2D states which is robust against details of quantized field flux and explains the occurrence of such states only at specific fractions for fillings, surprisingly coinciding for FQHE and for fractional Chern insulators.

To be more specific with this regard, the recent analyzes of FQHE in model systems without Landau levels [33] [34] are worth emphasizing also. In the paper [33] there is constructed a class of model Hamiltonians on 2D lattice which give nearly-flat bands with nontrivial topology. This property is regarded as a required prerequisite for organization of FQHE-like states when interaction would be next included. For flat band the kinetic energy is frozen which allows the interaction to dominate and create strongly correlated state of FQHE type. This has been theoretically verified in the paper [34] for a checkerboard lattice including nearest and next-nearest interaction in model Hamiltonian of the form,

, (7)

where H0 is a two-band checkerboard lattice model with nonzero Chern number implemented by complex hopping factors of the type,

, (8)

and H1 describes ordinary real-number-assigned hopping between next and next-next nearest neighbors [33] . Some attributes characteristic for FQHE have been indicated within this model for fractional fillings 1/3 and 1/5 (in the latter case repulsion V was required above a certain threshold value, unless U enhances strongly) [34] . This observation supports an idea of multi-looped structure of quasiclassical wave packets which in this way can reach equidistantly separated 2D particles (in every third cell for) due to repulsion interaction in almost flat band with suppressed kinetic energy, quite similarly as in the described above 2DEG system in the magnetic field. Though any links can be here drawn toward CF model with auxiliary magnetic field flux quanta attached to hypothetical composite particles, the multi-looped requirements in order to enhance orbits still hold. As number of loops can be only integer, this explains the fractional structure of fillings exactly in the same manner as in the case of 2DEG upon strong magnetic field. The role of cyclotron orbit quantization is substituted here by the orbit quantization due to Chern number invariant conservation (i.e., the quantization of the Berry field flux instead of the magnetic field flux).

6. Conclusions

By means of braid group approach it is possible to select appropriate braid subgroups of the full braid group of which one dimensional unitary representations (1DURs) define effective particles in the correlated states referred to FQHE. The argumentation is linked with the simple observation that at fractional fillings of the LLL the cyclotron trajectories which build braids in equidistantly distributed 2D charged system are too short in comparison to particle separation when the magnetic field is sufficiently strong. This precludes particle exchanges which is, however, necessary for organization of the collective multiparticle state with the determined statistics according to 1DURs of related braid group. One can observe that only at these filling fractions at which FQHE occurs the multi-looped braid structure recover exchanges along enhanced cyclotron trajectories. This enhancement is an exclusive property of 2D system when additional loops of cyclotron trajectory cannot add a surface (oppositely to 3D multi-looped trajectory), but must share the same total external magnetic field flux, which leads to effective enlargement of cyclotron orbits. For fillings of the LLL, the braid trajectories must be q-looped and then corresponding cyclotron orbits match neighboring particles without any artificial constructions. This unavoidable property of braids directly gives Laughlin correlations in the natural way and simultaneously explains the underlying spirit and structure of composite fermions phenomenologically introduced to illustrate Laughlin correlations. The flux tubes attached to composite fermions do not actually exist and they model the result of additional cyclotron loops presence. Recently developed theoretical studies of the fractional Chern insulators support correlated states with similar fractional hierarchy as in FQHE but without any magnetic field. This apparently goes beyond the explanation ability of the standard CF concept due to absence of the magnetic field in such systems, but still admit the multi-looped braid group explanation. Instead of the magnetic field quantization in fractional topological Chern insulators one can consider quantization of the Berry field flux which selects orbits similarly to magnetic field flux quantization. Multi-looped trajectories are here responsible for the same hierarchy of fillings as in FQHE. This evidences some advantages of the homotopy braid group approach to correlations in various 2D systems.

Acknowledgements

The support from the NCN Project UMO-2011/02/A/ST3/00116 is acknowledged.

References

  1. Ryder, L.H. (1996) Quantum Field Theory. 2nd Edition, Cambridge University Press, Cambridge. http://dx.doi.org/10.1017/CBO9780511813900
  2. Spanier, E. (1966) Algebraic Topology. Springer-Verlag, Berlin.
  3. Hatcher, A. (2002) Algebraic Topology. Cambridge University Press, Cambridge.
  4. Mermin, N. (1979) The Topological Theory of Defects in Ordered Media. Reviews of Modern Physics, 51, 591. http://dx.doi.org/10.1103/RevModPhys.51.591
  5. Prodan, E. (2011) Disordered Topological Insulators: A Non-Commutative Geometry Perspective. Journal of Physics A: Mathematical and Theoretical, 44, Article ID: 113001. http://dx.doi.org/10.1088/1751-8113/44/11/113001
  6. Hasan, M.Z. and Kane, C.L. (2010) Colloquium: Topological Insulators. Reviews of Modern Physics, 82, 3045-3067.
  7. Qi, X.L. and Zhang, S.C. (2011) Topological Insulators and Superconductors. Reviews of Modern Physics, 83, 1057. http://dx.doi.org/10.1103/RevModPhys.83.1057
  8. Thouless, D.J., Kohmoto, M., Nightingale, M.P. and den Nijs, M. (1982) Quantized Hall Conductance in a Two- Dimensional Periodic Potential. Physical Review Letters, 49, 405. http://dx.doi.org/10.1103/PhysRevLett.49.405
  9. Berry, M.V. (1984) Quantal Phase Factors Accompanying Adiabatic Changes. Proceedings of the Royal Society of London. Series A, Mathematical and Physical Sciences, 392, 45-57.
  10. Nakahara, M. (1990) Geometry, Topology and Physics. Adam Hilger, Bristol.
  11. Birman, J.S. (1974) Braids, Links and Mapping Class Groups. Princeton University Press, Princeton.
  12. Laidlaw, M.G. and DeWitt, C.M. (1971) Feynman Functional Integrals for Systems of Indistinguishable Particles. Physical Review D, 3, 1375-1378. http://dx.doi.org/10.1103/PhysRevD.3.1375
  13. Jacak, J., Jóźwiak, I. and Jacak, L. (2009) New Implementation of Composite Fermions in Terms of Subgroups of a Braid Group. Physics Letters A, 374, 346-350. http://dx.doi.org/10.1016/j.physleta.2009.10.075
  14. Jacak, J., Jóźwiak, I., Jacak, L. and Wieczorek, K. (2010) Cyclotron Braid Group Structure for Composite Fermions. Journal of Physics: Condensed Matter, 22, Article ID: 355602. http://dx.doi.org/10.1088/0953-8984/22/35/355602
  15. Pan, W., Störmer, H.L., Tsui, D.C., Pfeiffer, L.N., Baldwin, K.W. and West, K.W. (2003) Fractional Quantum Hall Effect of Composite Fermions. Physical Review Letters, 90, Article ID: 016801. http://dx.doi.org/10.1103/PhysRevLett.90.016801
  16. Laughlin, R.B. (1983) Anomalous Quantum Hall Effect: An Incompressible Quantum Fluid with Fractionally Charged Excitations. Physical Review Letters, 50, 1395-1398. http://dx.doi.org/10.1103/PhysRevLett.50.1395
  17. Haldane, F.D.M. (1983) Fractional Quantization of the Hall Effect: A Hierarchy of Incompressible Quantum Fluid States. Physical Review Letters, 51, 605-608. http://dx.doi.org/10.1103/PhysRevLett.51.605
  18. Prange, R.E. and Girvin, S.M. (1990) The Quantum Hall Effect. Springer-Verlag, New York. http://dx.doi.org/10.1007/978-1-4612-3350-3
  19. Laughlin, R.B. (1983) Quantized Motion of Three Two-Dimensional Electrons in a Strong Magnetic Field. Physical Review B, 27, 3383-3389. http://dx.doi.org/10.1103/PhysRevB.27.3383
  20. Landau, L.D. and Lifshitz, E.M. (1972) Quantum Mechanics: Non-Relativistic Theory. Nauka, Moscow.
  21. Abrikosov, A.A., Gorkov, L.P. and Dzialoshinskii, I.E. (1975) Methods of Quantum Field Theory in Statistical Physics. Dover Publications Inc., Dover.
  22. Jain, J.K. (1989) Composite-Fermion Approach for the Fractional Quantum Hall Effect. Physical Review Letters, 63, 199-202. http://dx.doi.org/10.1103/PhysRevLett.63.199
  23. Wilczek, F. (1990) Fractional Statistics and Anyon Superconductivity. World Scientific, Singapore City. http://dx.doi.org/10.1142/0961
  24. Wu, Y.S. (1984) General Theory for Quantum Statistics in Two Dimensions. Physical Review Letters, 52, 2103-2106. http://dx.doi.org/10.1103/PhysRevLett.52.2103
  25. Sudarshan, E.C.G., Imbo, T.D. and Govindarajan, T.R. (1988) Configuration Space Topology and Quantum Internal Symmetries. Physics Letters B, 213, 471-476. http://dx.doi.org/10.1016/0370-2693(88)91294-4
  26. Avron, J.E., Osadchy, D. and Seiler, R. (2003) A Topological Look at the Quantum Hall Effect. Physics Today, 56, 38- 42.
  27. Qi, X.L. and Zhang, S.C. (2010) The Quantum Spin Hall Effect and Topological Insulators. arXiv:1001.1602v1 [cond-mat.mtrl-sci]
  28. Wang, Z., Qi, X.L. and Zhang, S.C. (2010) Topological Order Parameters for Interacting Topological Insulators. Physical Review Letters, 105, Article ID: 256803. http://dx.doi.org/10.1103/PhysRevLett.105.256803
  29. Qi, X.L. (2011) Generic Wave-Function Description of Fractional Quantum Anomalous Hall States and Fractional Topological Insulators. Physical Review Letters, 107, Article ID: 126803. http://dx.doi.org/10.1103/PhysRevLett.107.126803
  30. Haldane, F.D.M. (1988) Model of Quantum Hall Effect without Landau Levels: Condensed Matter Realization of the “Parity Anomaly”. Physical Review Letters, 61, 2015-2018. http://dx.doi.org/10.1103/PhysRevLett.61.2015
  31. Kourtis, S., Venderbos, J.W.F. and Daghofer, M. (2012) Fractional Chern Insulator on a Triangular Lattice of Strongly Correlated t2g Electrons. Physical Review B, 86, Article ID: 235118. http://dx.doi.org/10.1103/PhysRevB.86.235118
  32. Parameswaran, S.A., Roy, R. and Sondhi, S.L. (2013) Fractional Quantum Hall Physics in Topological Flat Bands. Comptes Rendus Physique, 14, 816-839. http://dx.doi.org/10.1016/j.crhy.2013.04.003
  33. Sun, K., Gu, Z., Katsura, H. and Das Sarma, S. (2011) Nearly Flatbands with Nontrivial Topology. Physical Review Letters, 106, Article ID: 236803. http://dx.doi.org/10.1103/PhysRevLett.106.236803
  34. Sheng, D.N., Gu, Z.C., Sun, K. and Sheng, L. (2011) Fractional Quantum Hall Effect in the Absence of Landau Levels. arXiv:1102.2658v1 [cond-mat.str-el]

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