By Emil Prodan

ISBN-10: 3319293508

ISBN-13: 9783319293509

ISBN-10: 3319293516

ISBN-13: 9783319293516

This monograph deals an outline of rigorous effects on fermionic topological insulators from the complicated periods, specifically, these with out symmetries or with only a chiral symmetry. specific concentration is at the balance of the topological invariants within the presence of robust sickness, at the interaction among the majority and boundary invariants and on their dependence on magnetic fields.

The first half provides motivating examples and the conjectures recommend by way of the physics group, including a short assessment of the experimental achievements. the second one half develops an operator algebraic procedure for the research of disordered topological insulators. This leads clearly to using analytical instruments from K-theory and non-commutative geometry, resembling cyclic cohomology, quantized calculus with Fredholm modules and index pairings. New effects comprise a generalized Streda formulation and an evidence of the delocalized nature of floor states in topological insulators with non-trivial invariants. The concluding bankruptcy connects the invariants to measurable amounts and therefore provides a cultured actual characterization of the advanced topological insulators.

This e-book is meant for complicated scholars in mathematical physics and researchers alike.

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**Example text**

In other words, the only way to cross from the topological to the trivial phase is to go through a localization-delocalization quantum transition. As we shall see, it is exactly this divergence of the localization length which triggers an abrupt change in the quantized values of the bulk topological invariant. While the bulk analysis, just by itself, can be carried in the regime of strong disorder, the bulk-boundary correspondence will be established under the following assumption: / σ (Hω ). 2), that is JHω J = − Hω , and therefore also the flat band Hamiltonian Qω = 1 − 2Pω = sgn(Hω ) satisfies JQω J = −Qω and Qω2 = 1.

16) are sometimes also called Dirac points, which is not appropriate for the following reasons. t. the product γ1 · · · γd . This splits it into two chiral sectors and, in each of those chiral sectors, one gets the classical Weyl operator k, σ when the “time” direction is separated out. Here, γ and σ denote the Dirac and Pauli matrices. This pattern can be recognized in any dimension, and in general, the Weyl operator involves an odd number of Clifford generators and does not have a chiral symmetry, but rather a chirality that will be introduced below.

21). This implies Ch1 (u) = Ch1 (u0 ) for u ∈ C 1 (A1 ). 4) as a winding number. In particular, this shows that Ch1 (u) ∈ Z. An alternative way to verify the integrality of Ch1 (u) is to prove an index theorem. This has the advantage that one can also prove that the pairing is well-defined and integral in the regime of a mobility bulk gap, namely, when the Fermi level lies in a region of the essential spectrum which is dynamically Anderson localized. This type of extension is crucial for the understanding of the quantum Hall effect [20] and will be discussed further in Chap.

### Bulk and Boundary Invariants for Complex Topological Insulators: From K-Theory to Physics by Emil Prodan

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