Topolectrical circuits

Invented by Alessandro Volta and F\'elix Savary in the early 19th century, circuits consisting of resistor, inductor and capacitor (RLC) components are omnipresent in modern technology. The behavior of an RLC circuit is governed by its circuit Laplacian, which is analogous to the Hamiltonian describing the energetics of a physical system. We show that topological semimetal band structures can be realized as admittance bands in a periodic RLC circuit, where we employ the grounding to adjust the spectral position of the bands similar to the chemical potential in a material. Topological boundary resonances (TBRs) appear in the impedance read-out of a topolectrical circuit, providing a robust signal for the presence of topological admittance bands. For experimental illustration, we build the Su-Schrieffer-Heeger circuit, where our impedance measurement detects a TBR related to the midgap state. Due to the versatility of electronic circuits, our topological semimetal construction can be generalized to band structures with arbitrary lattice symmetry. Topolectrical circuits establish a bridge between electrical engineering and topological states of matter, where the accessibility, scalability, and operability of electronics synergizes with the intricate boundary properties of topological phases.

Topological semimetals 1 constitute the latest development of an evolution dating back more than thirty years, when topological phases began to cast their shadows before as midgap states in polyacetylene 2 and the quantized edge modes of integer quantum Hall systems 3 were discovered. Driven by the flourishing field of topological insulators 4,5 , the viewpoint of topology has recently branched out to various classes of physical systems, ranging from electrons in solids to photonic networks in metamaterials, ultra-cold atoms in optical lattices, microwave resonators, electrical circuits, and phonons in mechanical setups (see e.g. Refs. [6][7][8][9][10][11]. Note that such topological states of matter do not necessarily rely on any quantum mechanical framework. In mathematical terms, it is not the quantum, i.e. non-commutative, nature of the Hilbert space, but rather the non-trivial connectivity of phase space under cyclic evolution of parameters 12 that indicates a topological phase.
The fingerprint of a topological insulator motif, independent of the physical setting in which it is realized, is given by a single edge mode response protected by topology, along with an unresponsive bulk. While there are various promising approaches to realize them within classical arrays, topological device design is often limited due to insufficient edge mode density. As opposed to fermionic systems where the chemical potential is a useful parameter to access any particular range of the band structure at low energies, bosonic or classical degrees of freedom for a topological band structure also pose the problem how to systematically address the spectral regime of interest, such as the band gap domain of a topological insulator. Furthermore, in an era where classical experimental setups for topological phases still need to improve in terms of uniformity of array elements, it is often challenging to resolve single edge mode responses to identify the onset of a topological insulator phase.
We propose the topological semimetal paradigm in classical 2) of an illustrative RLC circuit with nodes {a, b, c}. W and D are diagonal matrices containing the total conductances from each node towards the ground and towards the rest of the circuit, respectively. C is the adjacency matrix of the circuit graph, with edges weighted by their conductances.
RLC circuits, which predicts highly pronounced resonances in a generic impedance read-out whenever there are topological boundary modes that scale extensively, such as the Fermi arcs of topological semimetals 13 . Due to their extensive degeneracy, such topological boundary resonances (TBRs) remain robust even in the face of significant nonuniformity of circuit elements, promising highprecision identification in a realistic measurement. We outline a detailed design of such topolectrical circuits, including a Weyl circuit network exhibiting TBRs of Fermi arc type, where the AC driving frequency combined with the grounding design takes over the role of the chemical potential in a fermionic system. As an initial proofof-principle experimental study, we report impedance and voltage profile measurements of the Su-Schrieffer-Heeger circuit chain. As a theoretical byproduct in this work, we further introduce the mathematical framework for characterizing topological properties of electrical circuit graphs in general. While our semimetal paradigm can be applied to any classical array setup such as mechanical systems or optical cavities, the topolectrical circuits we introduce combine all desired conceptual and experimental preferences to realize topological semimetal analogs in a classical model, without demanding specialized equipment.
Any electrical circuit network can be represented by a graph whose nodes and edges correspond to the circuit junctions and connecting wires/elements. The circuit behavior is fundamentally described by Kirchhoff's law where Ia and Va are the input current and electrical potential at each node a. By current conservation, Ia equals the total current flowing out of node a towards all other nodes i linked by nonzero conductance Cai, plus the current flowing into the ground through a route with impedance w −1 a . The impedance and conductances are real for An AC source provides a driving voltage with amplitude V0. For t = C1/C2 < 1, an SSH midgap mode is found. In the experimental implementation we set C1 = 0.1µF, C2 = 0.22µF and L=10µH. Green lines indicate wiring for measuring the t −1 -configuration on the same circuit. (b) Ideal impedance magnitude across the nodal ends a = 1 and b = N of an N = 10 SSH topolectrical circuit as a function of AC frequency ω for various values of t. The dashed curves highlight topologically trivial cases for t > 1, showing that the impedance increases enormously only for t < 1, the topologically nontrivial regime. The TBR at ω =ω is most pronounced for the smallest t, and decreases exponentially as t is increased. Secondary resonances are observed at larger deviations fromω, and are associated with other eigenvalues of the grounded circuit Laplacian J. (c) Measurement of ψ0(n), which accurately fits the shape predicted by theory, i.e., ψ0(n) = ((−t) n V0, 0) for the nth two-site unit cell from the left, see also (a) for node numbering. (d) Impedance measurement of the t = 0.22 and t −1 = 4.5 configuration. Despite non-negligible serial resistances and element non-uniformities, the SSH midgap peak is clearly observed in the impedance measurement and absent for the t −1 = 4.5 configuration.
resistive circuit elements, but will be complex when capacitors or inductors are present (Fig. 1). As an initial step towards identifying circuits with tight-binding lattice models, we rewrite Eq. 1 in compact matrix form with vectors V and I formed by the components Va and Ia. The grounded Laplacian J consists of L, the circuit Laplacian which depends on the conductance network structure, and W = diag(w1, w2, . . . ), which depends on how the circuit is grounded. The Laplacian is defined in terms of the conductances by L = D − C, where C is the (adjacency) matrix of conductances and D = diag( i C1i, i C2i, . . . ) lists the total conductances out of each node (Fig. 1). To understand the relation of L with the continuum Laplacian, one writes the spreading of current from a node as a divergence of current density I = ∇ · j, and invokes the definition of conductivity j = σE = σ∇V . Hence I = ∇ · (σ∇)V = LV. This establishes L as the continuum Laplacian restricted to a circuit.
A circuit is most commonly studied through an impedance measurement, which involves running a current through it and measuring the voltage response. As capacitive and inductive resistances explicitly depend on it, the driving voltage frequency ω is a central tuning parameter of topolectrical circuits. The simplest measurement is the two-point impedance Z ab = (Va − V b )/I between nodes a and b, where Va − V b is their potential difference and I is the magnitude of the current I a,b = ±I that enters at a and leaves at b. To determine Z ab , the potentials have to be expressed in terms of the input current by inverting Eq. 2. For this purpose, we employ the regularized inverse of J known as the circuit Green's func-tion G = jn =0 1 jn ψ n ψ † n , where jn and ψn denote the admittance eigenvalues and the N -dimensional eigenmode vectors of J, respectively. (Regularization in this context means that jn = 0 modes are omitted when the circuit is not grounded (W = 0) and hence defined up to an overall potential offset. If J is not Hermitian, ψ † n and ψn are replaced by the left and right eigenvectors.) The eigenmodes are potential distributions proportional to the input current distribution. Note that G is always symmetric when the circuit elements are reciprocal (see also Ref. 14). The two-point impedance reads 15 where ψn,a − ψ n,b is the difference between the amplitudes of the nth admittance eigenmode. As such, the impedance for each mode n depends on the squared magnitude of its potential difference between a and b, weighted by its eigen-impedance j −1 n . To make contact with topological bandstructures, we consider circuits made up of periodic sublattices. A node a = (x, s) can be indexed by its unit cell position x and sublattice label s. Due to translation symmetry, Bloch's theorem allows us to index the eigenmodes by momentum k and band index m, i.e. ψ (k,m) (x, s) = ϕm(k, s)e ik·x . Henceforth, we shall call the set of eigenvalues j k,m the bandstructure of the circuit, and also refer to the nodes as sites. The impedance between two sites (0, s) and (x, s ) takes the form which reduces to k,m 4j −1 k,m |ϕm(k, s)| 2 sin 2 k·x 2 for nodes on the same sublattice s = s . The impedance between two nodes becomes large if there exists a finite density of nontrivial eigenmodes with small j k,m . Such divergences correspond to resonances in RLC circuits, and will be even more pronounced if the relevant eigenmodes are localized at one region, e.g. a boundary of the circuit or a domain wall trajectory. This is the case for TBRs in topolectrical circuits, where there exists a large density of protected boundary modes with j k,m ≈ 0. A central result of our work will be the construction of such topolectrical circuits with "grounded" RLC networks, with the ground controlling the pinning of the TBR to j k,m ≈ 0.
The most elementary 2-band topolectrical circuit can be built from a line of capacitors with alternating capacitances of C1 and C2 (Fig. 2), which is characterized by t := C1/C2. Note that as will be relevant in the following, changing the initial capacitor to the left from C1 → C2 implies t → 1/t. Identical inductors L connect the junctions between each capacitor to a common isolated grounding plate. For t < 1, a topological boundary mode exists and leads to a drastic increase in circuit impedance, i.e., a TBR. Consider one setup of Fig. 2, with the leftmost grounded capacitor of capacitance C1 < C2, and another setup with C1,2 interchanged. To see that the former arrangement supports a localized "midgap" eigenmode (configuration of potentials) that decays exponentially to the right, while the latter does not, notice that a fixed amount of charge Q between any pair of C1, C2 capacitors leads to potential differences V1, V2 related by Q = C1V1 = C2V2 between their respective plates. For t < 1, there will be a larger potential difference between the plates of C1 than that of C2. Indeed, when driven by an AC supply, V1 and V2 oscillate in anti-phase with relative amplitude V2/V1 = t, corresponding to the potential configuration ψ0(n) ∝ (1, 0, −t, 0, t 2 , 0, −t 3 , 0, ..., (−t) 2n+1 ), where the index n runs through all nodes. ψ0(n) is exponentially localized at the left end, with a decay length of ξ = (log C 2 C 1 ) −1 = − log t. Since V and the source/sink current I vanish on the even nodes and are proportional to (−t) 2n+1 on the odd nodes, it follows that ψ0 ≡ V ∝ I, i.e., ψ0 is an eigenmode of J.
In the language of the grounded circuit Laplacian, the system with periodic boundary conditions is described by which, up to prefactors, is equivalent to the enigmatic Su-Schriffer-Heeger (SSH) model developed for midgap states in polyacetylene 2 .
Here, σx and σy are the Pauli matrices defined in the basis consisting of a C1 capacitor and an adjacent C2 capacitor on its right. The boundary mode ψ0(x), where the notation x is now highlighting the site instead of the node interpretation n, is the circuit analog of the SSH zero mode consisting of "dimerized" pairs of capacitors with large amounts of charge oscillating between them. It is topologically protected by a 1D winding number (cf. appendices). For t < 1, one finds a nonzero topological winding which cannot be deformed into a trivial winding unless the gap, i.e., the spectral gap of the circuit Laplacian, closes.
Since the left end of the circuit by itself always marks the transition to a trivial regime, for t < 1 we expect a boundary mode with vanishing spectral value j0 in the semi-infinite limit. Indeed, as shown in the appendix, j0 ∼ (−t) N , where N denotes the total number of capacitors. This vanishing eigenvalue marks the TBR, which for open boundary conditions and a hypothetically ideal circuit without serial resistance is characterized by a divergent (Fig. 2b), whereω denotes the resonant frequencyω = 1/ L(C1 + C2), and da, d b are the unit cell distances of nodes a and b from the leftmost capacitor.
The theoretical prediction described above is rather precisely what we find experimentally. In the setup depicted in Fig. 2a, we can switch between a capacitor ratio of t and 1/t depending on how fix the switch to node 1 or 2, which affects the boundary condition where the external voltage source is applied. No midgap mode at the external voltage frequencyω is observed for t > 1, but for t < 1. For experimental convenience, we have constrained ourselves to measuring the impedance at the pair of nodes at the boundary, and further map out the midgap voltage profile eigenstate ψ0(n) of the circuit by measuring the voltage difference between neighboring nodes (Fig. 2c,d). ψ0(n) displays the predicted behaviour within negligible error bars. We find the latter to be a robust measurement, along with the predicted impedance profile if we allow for non-uniformity of circuit elements and consider serial circuit resistance in our calculations (cf. appedices).
A more targeted TBR response at the boundaries can be achieved in higher-dimensional topolectrical circuits, where the increased admittance density of states (DOS) from an additional dimension makes it possible to spatially isolate the topolectrical resonance. The SSH circuit can be straightforwardly extended to represent a 2D band structure by adding a spatial modulation to the capacitances with inverse wavelength ky along a new direction, such that a phase transition at t = 1 occurs at a certain range of ky. This can be achieved, for instance, through the parametrization C1 = γ + 2β cos ky, C2 = γ + 2α cos ky, bringing the grounded Laplacian to the form In real space, this 2D circuit consists of a lattice network with two inequivalent nodes per unit cell, where unlike nodes are connected by capacitors of capacitances α, β, or γ depending on their relative orientations (Fig. 3). Each node is also connected to the ground by an inductor L. The two-site unit cell, along with the lattice connectivity and edge termination, provides a circuit analog of the zigzag (ZZ) edge of graphene 16 . This circuit network supports topological boundary modes inherited from its SSH predecessor. If we ground the capacitors on one/both of its edges perpendicular to the x-direction, but leave the circuit periodic in the y-direction by connecting the last capacitor with the first capacitor, a line of singly/doubly degenerate edge modes appear for ky satisfying t < 1, i.e. (α − β) cos ky > 0. , these edge modes correspond to an extensive line of vanishing eigenvalues j0 that dramatically enhance the circuit impedance at the edge. This can be physically explained in terms of edge resonances involving isolated triplets of simultaneously "dimerized" capacitors sharing oscillating charges, reminiscent of those in the SSH topolectrical circuit. When α > β and |ky| < π/2, the capacitors in horizontally adjacent unit cells collectively "dimerize" by harboring strongly oscillating charges. Reversing the former condition to α < β makes the dimerization incompatible with the edge grounding, while breaking the condition |ky| < π/2 also inhibits these oscillations by reversing the relative polarity of adjacent capacitors. Since this dimerization ultimately relies on sublattice symmetry, the TBR only appears when the edges respect sublattice symmetry, such as in the zigzag case. A realistic implementation is illustrated in Fig. 3, where a fixed realistic serial resistance is attached to each grounding wire. Z ss x 1 ,x 2 denotes the impedance between the sth node of unit cell x1 = (x1, y1) and the s th node of unit cell x2 = (x2, y2), s, s ∈ {A,B}, the left edge being located at x = 0 (cf. appendices for detailed calculations). Topologically, the circuit is a cylinder periodic in y-direction, with a circumference of Ly rows. As plotted in Fig. 3d for A-type nodes, the impedances in both x and y directions (Z AA (x 1 ,0),(x 2 ,0) and Z AA (x,0),(x,y) ) are greatly enhanced only near the edge, in contrast to the previous 1D SSH circuit. This enhancement is apparent even for short intervals, as reflected by the rapid rise of impedance Z AA (x,0),(x,y) at small y. For circuits representing higher dimensional band structures, a deeper consequence of Eq. 4 is that the TBR depends on the scale set by the maximal imaginary gap 17 , even if the boundary modes themselves are gapless and algebraically decaying. This conundrum is addressed in the appendix.
Along these Fermi arcs, we recover the line nodes of the zigzag topolectrical circuit, where the massive degeneracy is protected by sublattice symmetry.
Topolectrical circuits can be realized using basic laboratory equipment. For a realistic implementation, however, as we have also seen for our experimental implementation of the SSH circuit, one has to take into account the non-uniformity of RLC components, as well as capacitive and resistive losses. We find that topolectrical circuits, which are analogous to topological semimetals, are markly superior to e.g. topological insulator circuits in this respect, as shown in Fig. 4c,d. There, we compare the impedance read-out of our topolectrical circuits containing extensive mode degeneracy (Eqs. 6 and 7) with that of a topological insulator circuit 8,18 , which we adjusted by grounding it with inductors such that both systems can be accurately tuned for possible TBRs through the AC frequency (cf. appendices). Due to the extensively large boundary DOS which is broadened but not destroyed by disorder (Fig. 4c), sharply defined topolectrical resonances exist e.g. in the Weyl or zigzag circuit, even with 10% error tolerance in each circuit element. Furthermore, due to extensivity, the resonances remain pronounced even when disorder shifts them slightly away fromω, i.e. the resonant frequency at zero disorder. By contrast, the impedance resonance peaks of the topological insulator circuit are neither as pronounced nor immune to disorder, since they are mostly due to the bulk modes. Although their boundary modes are likewise topologically protected, they exist at isolated momenta at any given frequency, and thus have limited contribution to the impedance read-out. We find, however, that the voltage eigenstate profile ψ0(n), as we have measured it for the SSH midgap mode, is still accessible, and thus is one of the most sensible quantities to measure for topological insulator circuits. From a broader point of view on 3D topolectrical circuits, the requisite Fermi arcs for TBRs can occur in the presence of more exotic symmetries, e.g. certain non-symmorphic symmetries appearing in known Weyl semimetals or photonic crystals 19 . Many of these symmetries, and hence their accompanying topological phases, can be conveniently realized in electrical circuits, whose network structure is free from physical limitations imposed by the shape of ionic orbitals. Topolectrical circuits are likewise not restricted by intrinsic lengths scales from quantum mechanics, and can be constructed at macroscopic sizes with connections across arbitrarily distant nodes. In particular, topolectrical circuits can be used to simulate higherdimensional topological phases without involving synthetic dimensions, since each node can be connected to other nodes along more than three axes (Fig.4e). The ability to go beyond a regular periodic structure also allows for an accessible study of topological phases on aperiodic networks 20 (Fig.4e) or hyperbolic lattices of arbitrary complexity 21,22 . Circuit elements such as capacitors can also be mechanically manipulated to break time-reversal symmetry, and induce novel non-equilibrium (Floquet) Chern phases 23 . In general, the TBR can also be designed to appear not at the physical boundary of the circuit, but at domain walls along an arbitrary trajectory through the circuit (Fig.4e). For the zigzag circuit, such a formulation would bear strong similarity to flux lattice domain walls 24 . This domain wall design would certainly be of interest not just for topolectrical circuits, but also for mechanical systems. Method Section (Appendices) for "Topolectrical Circuits" Appendix A: Impedance formulae for 2-component periodic circuits It is instructive to explicitly evaluate Eq. 4 for general 2-node unit cell circuits for periodic boundary conditions (i.e. without grounded terminations). We start from where k denotes momentum, and ϕm are the eigenvectors of J(k) = d0(k) + d(k) · σ, with σ being the vector of Pauli matrices. In closed form, the impedances between nodes of sublattices A, B separated by x unit cells are given by (withd = d/|d|)

Appendix B: Circuit Green's function
A physical interpretation of G = J −1 as the inverse of a graph Laplacian is readily obtained. Write J = D + W − C, where [D] ab = δ ab c Cac is the diagonal matrix of the conductances emanating from each node towards other nodes, [W ] ab = δ ab wa the conductance of each node towards the ground, and C the adjacency matrix of the conductances. Then i.e. G ab is the number of paths of any length from node a to b, each weighted by the conductance ratio (i.e. transition probability) [(D + W ) −1 C] kl = C kl /(w k + l C kl ) between each pair of nodes k, l along the path. In other words, G keeps track of the fraction of the current that will flow between two nodes, assuming that it spreads out at each node it passes by. The simplest topolectrical circuit can be written out in explicit but still compact detail. From Kirchhoff's law, we can write the grounded Laplacian as with the last diagonal entry containing C1, C2 or both depending on which type of capacitor (or both) is connected to the rightmost node.
When ω is set to the resonant frequencyω = , the diagonal terms proportional to the identity disappear, and J possesses an exact expression for its inverse which is given by For C1/C2 = t < 1, there exists a boundary mode near (1 + t) 1 −ω 2 ω 2 , the middle of the bulk spectral gap of J SSH . Its eigenvalue j0 can be obtained from the characteristic polynomial of J SSH . At resonant frequency ω =ω, j0 is very close to zero, and we can neglect all but the linear term of the characteristic polynomial to obtain which exponentially decays with N , the number of capacitors in the SSH circuit. From Eq. 3 and ψ0 ∝ (1, 0, −t, 0, t 2 , ...), the impedance between nodes 1 and 2x − 1 (or 2x) is thus given by both of which are plotted in Fig. 2. Note that had C2 been instead greater than C1, ψ0(x) will not be have been able to exist as an eigenmode due to incompatible boundary conditions. However, if the right end of the circuit is also connected to a grounded capacitor C2, there can be another mirror-reflected, but otherwise identical, boundary mode localized on the right end.
To find the momentum space representation of the grounded Laplacian, we impose periodic boundary conditions and Fourier transform Eq. C1 to obtain as also presented in the main text.
From Eq. C6, it can be shown that for t < 1, J possesses gapped translation-invariant eigenmodes with eigenvalues j kx,± = C1 + C2 − 1 ω 2 L ± C 2 1 + C 2 2 + 2C1C2 cos kx. As follows from Eq. C3, there is also a midgap boundary mode with the eigenvalue which is not small when away from resonance. The SSH circuit has the special property that the decay length ξ = log C 2 C 1 of its boundary mode coincides exactly with the imaginary gap 17,25 , which is the imaginary part of kx necessary for closing the gap: On hindsight, the TBR of the SSH circuit has an elementary interpretation: Due to the special potential profile of the boundary mode (Fig.  2), a driving input voltage V0 and current I0 is connected to two capacitors and one inductor, all of which are at zero potential (grounded) at the other end. From the special decaying potential profile, the potential towards the far right (call it node b) must have vanishing potential. By Kirchhoff's law,

Sublattice symmetry (Z2) and SSH winding number
Eq. C6 is a map from S 1 to S 1 , and is characterized by an integer winding number The second step of Eq. C9 relies on the absence of a σz term in J SSH (kx), which is enforced by the sublattice symmetry of the circuit (every node looks the same up to a left-right reflection). This winding woul not be well-defined if, for instance, different inductors were connected to different nodes. This winding number N1D is related to the Chern number in the following sense. Consider a 2D extension to J SSH (Eq. C6). The contribution to N2D from a reciprocal space region R is given by where ∇ × A is the Berry flux. Now suppose there is sublattice symmetry, i.e. that there is no σ3 term so that d ⊥ê3. Then the second line reduces to a line integral along the equator of the bloch sphere, which is mathematically known as S 1 . Consequently, we can define a one-dimensional topological invariant of the winding of the mapping from the 1D torus ∂R to the equator S 1 → S 1 , as we did above. This invariant needs the protection of sublattice symmetry; upon breaking it by adding a small σ3 term, the d vector will not be confined to the equator, and a second homotopy invariant instead of a first homotopy invariant is required.

Realistic circuit calculation
With series resistance R on the inductor, which is the most relevant serial resistance to consider, we have the impedance of each inductor replaced by iωL → iωL + R. The grounded Laplacian is hence replaced by The TBR resonance peak occurs when the magnitude of the identity matrix term is as small as possible, i.e at the minimal value of which occurs at ω 2 =ω 2 = 1 L(C 1 +C 2 ) , as can be checked via finding the extremum of the above. For a resonance to occur at a nonzero real frequency, we will need α < 1 + √ 2 ≈ 2.41, while an accessible resonance realistically requires α < 10 −3 judging from our simulations. For R = 28 mOhm, L = 10 −5 H and C1 + C2 = 1.22 × 10 −7 F as given in our experimental setup, we have α ≈ 10 −5 , which is sufficiently small for a clean and visible resonance. Circuit element non-uniformities hardly have any detrimental effect on the SSH signal, as we checked up to 20% tolerance.

Experimental implementation
For the experimental implementation of the SSH-circuit a printed circuit board hosting ten unit cells was designed and fit with low serial resistance (< 26mΩ) inductors (Coilcraft MA5172-AE) and surface mount multilayer ceramic chip capacitors (Kemet 0805 / 1206), respectively. The circuit was fed by an arbitrary waveform generator (Agilent 33220A), the signals were picked up by lock-in amplifier (Zurich Instruments MFLI series).
In our notation, the simplest topological insulator circuit, which contains 3 capacitors per magnetic unit cell (Eq. 3 of Ref. 18), possesses the effective grounded Laplacian consisting of two copies (±) of −2 cos ky 0 0 0 −2 cos(ky ± 2π/3) 0 0 0 −2 cos(ky ∓ 2π/3) whereω 2 TI = 1 2C(L 1 +L 2 ) . Note that, opposite to our semimetal circuits, but in accordance to the convention in Ref. 18, the ungrounded elements are the inductors, not capacitors. This duplicity yields no extra complication, as the simple relation ω →ω 2 ω holds when the capacitors and inductors are interchanged. Eq. F1 is a variant of (2 opposite copies of) the 3-band Hofstadter Hamiltonian, with each copy possessing 3 bulk bands connected by topological edge modes. The crux is that although these are bona fide topologically protected modes, they do not necessarily contribute significantly to the RLC resonances because they cross a given eigenvalue only at isolated points in momentum space. According to our semimetal paradigm, TBRs are characterized by boundary modes that are (i) extensively degenerate and (ii) spatially localized, with the former not being satisfied by the TI circuit edge mode(s).
To study the precise implications of the absence of extensive degeneracy in a topolectrical circuit, we consider ensembles of disordered circuits, i.e. circuits consisting of elements with nonuniform capacitances C or inductances L. The nonuniformities are charactized by standard errors with tolerances (standard deviations) of 1% or 10%. Additionally, we have included resistive losses proportional to 10% of the non-uniformities of impedances due to disorder. The results are depicted in Figs. 4c and 4d. It becomes evident that the extensive, semimetal-like degeneracy of our Weyl circuit protects the RLC resonances much better than the protection from the single mode Kramer's degeneracy in the TI circuit. This observation identically holds for both the Weyl and zigzag topolectrical circuits.