Abstract
Kinetic helicity is one of the invariants of the Euler equations that is associated with the topology of vortex lines within the fluid. In superfluids, the vorticity is concentrated along vortex filaments. In this setting, helicity would be expected to acquire its simplest form. However, the lack of a core structure for vortex filaments appears to result in a helicity that does not retain its key attribute as a quadratic invariant. By defining a spanwise vector to the vortex through the use of a Seifert framing, we are able to introduce twist and henceforth recover the key properties of helicity. We present several examples for calculating internal twist to illustrate why the centreline helicity alone will lead to ambiguous results if a twist contribution is not introduced. Our choice of the spanwise vector can be expressed in terms of the tangential component of velocity along the filament. Since the tangential velocity does not alter the configuration of the vortex at later times, we are able to recover a similar equation for the internal twist angle to that of classical vortex tubes. Our results allow us to explain how a quasiclassical limit of helicity emerges from helicity considerations for individual superfluid vortex filaments.
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Introduction
Ideal classical fluids possess a number of conserved quantities such as energy, momentum, angular momentum and kinetic helicity. Of these, only energy and kinetic helicity correspond to quadratic invariants in the system. First identified as an invariant for ideal classical fluids by Moffatt^{1}, kinetic helicity has been recognized to be related to the topology of the vorticity field in classical fluids. Aside from its relevance to classical fluids, helicity also plays an important role in a number of other contexts such as plasmas, cosmic strings, magnetohydrodynamics, and biology^{2,3,4,5,6,7,8,9,10}.
If vorticity is concentrated within vortex tubes, the helicity is in part determined by the selfknotting and linking of the vortices within a tangle. In recent years, it has become possible to realize particular cases of knotted vortex tubes produced in water and to study them under controlled conditions in the laboratory^{11}. This has paved the way to test assertions arising from considerations involving helicity. Recently, tying a simple knot has been experimentally demonstrated in a spinor BoseEinstein condensate^{12}. Even though the characteristics of superfluid ^{4}He are different, similar knotted vortex excitations would be expected to arise. However, their experimental verification would be more of a challenge since it is only recently that direct visualization of quantized vortices in ^{4}He has become possible using small tracer particles^{13}.
In contrast to classical fluids, in superfluids, the vorticity is concentrated along line filaments and the circulation is quantized in units of Planck’s constant. Moreover, superfluid vortices are not subject to diffusive processes that are present in classical fluids. Yet, although superfluid vortices appear to resemble vortices of ideal classical fluids, their topology is not frozen into the flow because quantum effects can act to allow vortices to undergo reconnections. In other words, superfluid vortices are not constrained by the Helmholtz laws of vortex motion. Given these observations, it appears that helicity would acquire its simplest form in a superfluid. At the same time, reconnections delineate the boundaries of sharply defined intervals involving constant vortex topologies. This makes superfluids an ideal setting in which to understand properties of helicity and how it relates to the topology of the superfluid vortex filaments.
Numerical studies of knotted vortex structures have previously been performed using both a hydrodynamic description based on a vortex filament model^{14} and a microscopic mean field model in the form of the GrossPitaevskii equation that can directly resolve the core structure^{15}. In superfluids, the core of a vortex is characterised by a depletion of the density field which vanishes along the centreline of the vortex. Therefore, although superfluid vortices have a finite core size characterized by the rapid variation of the density field, the vorticity remains singular and concentrated along a filament due to the divergent nature of the velocity within the core. When the core size is much smaller than any other characteristic scale and compressiblity effects can be neglected, one may adopt a vortex filament model in which the dynamics of the superfluid reduces to studying how a vortex or a tangle of vortices evolves. Both these conditions are typically satisfied in ^{4}He. In this case, the vortex core size is of the order of 1 Å. Moreover, since superfluid helium is a liquid, it is much more reasonable to assume that it behaves as an incompressible fluid. The vortex filament model has served as an excellent description to study the dynamics of vortices in this system.
Since a vortex filament has no internal structure associated with the vorticity field, there is no notion of the twisting of the vortex lines within the core of a vortex as is the case for vortex tubes with a crosssectional area characterising the finite extent of the vorticity field. Such a scenario leads to a number of complications when evaluating helicity for a vortex filament. In particular, it would appear that helicity conservation can not be satisfied, even in between reconnection events.
In this work, we will show that without introducing the notion of an internal twist, helicity conservation can not be satisfied within the vortex filament model. To introduce internal twist, a spanwise vector must be defined along the length of the filament. We will show that a natural choice is to set the spanwise vector to coincide with a direction of constant velocity potential upon which we are able to recover the key properties of helicity. In superfluids the quantum mechanical phase of the order parameter plays the role of the velocity potential. We note that similar choices have been suggested also by other authors^{16,17,18,19}. We will illustrate that this choice of the spanwise vector coincides with working in the socalled Seifert frame in which case helicity becomes trivially zero^{20,21}. In this frame, the direction of the spanwise vector is related to the tangential component of the standard BiotSavart velocity along the vortex filament. When the filament is interpreted as a limiting case of a classical vortex tube endowed with internal structure, the tangential velocity of the vortex filament is modified. Since the tangential velocity does not affect the overall configuration of the vortices, our definition remains consistent with the vortex dynamics produced by the vortex filament model. This allows us to generalize our results for superfluid vortices to classical vortices. In particular, our results will allow us to establish how a quasiclassical limit of helicity can emerge from the microscopic quantum description.
Results
Helicity and its components
We will begin by recalling some key results concerning helicity in classical fluids. Helicity in fluid dynamics is defined as
where the integration is over the whole space where the flow is defined, v = v(r, t) is the velocity field, and is the corresponding vorticity field. If the vorticity is taken to be concentrated within vortex tubes but is zero otherwise, the helicity will have a topological interpretation. For simplicity, we will consider the scenario where each vortex tube carries the same vorticity flux κ. This flux can be identified with the circulation which for quantized vortices is given by κ = h/m. Here, h is Planck’s constant and m is the atomic mass (e.g. of the ^{4}He atom). Following Moffatt and Ricca^{22}, we decompose the helicity into the linking number (where the double summation is over different vortices and L_{ij} is the Gauss linking number), the writhe , and the twist part of the helicity such that
To provide more explicit expressions for these terms, we parameterize a vortex in terms of its arclength ξ so that the position vector of a vortex filament is given by s = s(ξ, t). It is then natural to introduce the FrenetSerret basis given by Eq. (3) to evaluate the curvature c(ξ, t), and torsion τ(ξ, t) of each vortex filament:
where and are local tangent, normal, and binormal (unit vectors), respectively. Here, primes imply differentiation with respect to arclength. Denoting the centreline of the vortex tube i with position vector s by C_{i}, we can then identify a unit spanwise vector N that determines the twisting of the vortex lines within the vortex tube such that
This vector can be attributed to a ribbon like structure that is oriented with respect to the unit normal and and binormal vectors. With these definitions, the different helicity components can be written as^{22,23}
The use of the FrenetSerret equations results in a twist contribution to the helicity that is given by
Here the torsion part of the twist T_{tors} can be evaluated using the local torsion τ(ξ). The last term in Eq. (6) describes the internal (or intrinsic) twist T_{tw}. We note that, since N is defined in terms of the normal and binormal unitvectors, a constant value of N only implies that the total twist is zero. The internal twist can still be nonzero if torsion is also nonzero.
For closed vortex tubes, both the Gauss linking number and the internal twist can only take integer values. The writhe, the Gauss linking number, and the torsion part of the twist do not depend on the way one prescribes the spanwise vector N. However, the internal twist depends on the choice for N^{24}. Nevertheless, once N is prescribed, the selflinking number for vortex i, which equals W_{i} + T_{i}, also becomes a topological invariant. It follows that by redefining N we may designate different values to the helicity.
Theoretically it has been shown that under continuous deformation of the vortex tube, writhe W and total twist T = T_{tors} + T_{tw} vary continuously. However, if at some time t = t_{c} a curve passes through an inflectional configuration, i.e., its curvature c(ξ) vanishes at some point ξ = ξ_{c}, then the torsion part of the helicity T_{tors} develops a jump of ±1. At the instant when the curve has a point with zero curvature, the local torsion, τ, diverges around ξ = ξ_{c}, but this divergence is integrable. The resulting jump is compensated by a jump in the internal twist of .
Helicity for vortex filaments
When the superfluid is described by a complex wavefunction (order parameter Ψ) then vorticity can arise only in the form of linelike topological defects. For pure line vortices (i.e. neglecting other excitations in the superfluid), the corresponding velocity potential φ can be identified with the phase of the order parameter such that . In this case, the phase is well defined everywhere, except at the vortex cores where the vorticity is nonzero.
If we ignore compressibility effects and focus on the incompressible motion given by the vortices that correspond to pure line defects, the superfluid velocity can be calculated using the standard BiotSavart law
where the integration is carried out along all the vortex lines. This equation can be directly applied at any point r ≠ s (i.e. not lying on a vortex). At a point r = s, the divergent integrand implies that the normal and binormal components of the velocity are not well defined at the vortex line. In contrast, the tangential component of v_{BS} remains wellbehaved. This difficulty can be circumvented by regularizing the integral in the vicinity of the point on a vortex as described in the Methods section.
If the BiotSavart integral is inserted into the Eq. (1) for the helicity, we appear to recover only the linking number and the writhe terms. Therefore, by using the above expression for the BiotSavart velocity it seems that the helicity is not the same as the one presented above.
Although a vortex filament has no internal core structure, on physical grounds a vortex is endowed with a scalar field, the velocity potential that permits us to identify a spanwise vector along a direction of constant phase. We note that in order to maintain full consistency throughout our formulation, it is important to work with the incompressible component of the phase (i.e. its divergence free projection). Therefore, whenever we refer to φ in what follows, we will assume this represents only this component of the phase. The direction of the constant phase (or velocity potential) of the complex wavefunction has also been proposed by others as a possible direction that can be used to define N for superfluid vortices^{16,17,18}. This choice for the vector N turns out to be equivalent to using the socalled Seifert framing. [Not all Seifert frames are equivalent to surfaces of constant phase. However, here we only consider those which correspond to a constant phase and use the term Seifert frame].
This particular framing is special because the total helicity is always zero when evaluated in this frame^{20,21}. With N as defined, it is now possible to recover a torsion and internal twist contribution to helicity. To see how this arises, we note that in the Seifert framing we have
where r* = s + εN represents a point located near a point s lying on the vortex. Here is proportional to the superfluid velocity, which is normal to surfaces of constant phase near a vortex. By construction, on the curve C* given by r = r* the phase is constant so that we can write φ(r*(ξ*)) = φ_{0}, where φ_{0} is an arbitrary constant. This implies that
where is the tangent for the curve C*. In the limit ε → 0, C* and C coincide and the tangent vector then approaches the tangent of the vortex line C. However, the above cannot be used to deduce that the tangential BiotSavart velocity along the vortex is zero. This is because, even if the azimuthal component (component around the vortex centreline) of goes to zero, the azimuthal component of the velocity diverges. Therefore, a more detailed analysis is required to determine the tangential velocity along the filament. By using the chain rule we can express as
After inserting the definition for N given by Eq. (4), and applying the FrenetSerret equations, plus noting that the local azimuthal direction around the vortex tangent is given by , the above equation for simplifies to
where describes the rate of rotation of the spanwise vector around the local tangent . In arriving at the final expression given in Eq. (11), we have assumed that the local curvature satisfies the condition , and we have used the unit normalization to determine the value for the common factor, dξ/dξ*.
We would expect that the leading order terms for the BiotSavart velocity at r = r* are given by
Now substituting Eqs (11) and (12) into Eq. (9) and taking the limit ε → 0, we obtain that
This implies that we may obtain the internal twist angle θ after calculating the tangential component of the BiotSavart velocity and the local torsion.
To clarify the relation between classical and quantum vortices, in order to establish how a quasiclassical limit can arise from the quantum case, let us consider the scenario of a classical vortex tube with a finite but small crosssectional area. As shown by Moffatt and Ricca^{22}, for a vortex with a finite core, it is possible to relate the twist of the vorticity flux lines to the twist of the spanwise vector in the equation for the helicity. Thus, in contrast to a quantum vortex, for a classical vortex, the twist T, defined in Eq. (6), originates from the azimuthal component of the vorticity.
In the case when the characteristic length scale along the vortex tube is much larger than the vortex core, it may be convenient to use the filament representation and study the dynamics of how the centreline vorticity evolves. However, this filament description of a vortex tube follows from a scale separation assumption rather than being an intrinsic representation of the actual vorticity field. A key difference with a superfluid vortex is that the internal vorticity structure now gives rise to a component of velocity along the centreline of the vortex tube. The total velocity for a vortex filament used to model a thin vortex tube is therefore given by
The additional tangential twist velocity arising from the twisting of the vortex flux lines is given by
Here τ(ξ) is the local torsion at ξ and N describes the rotation of the vorticity fluxlines inside the vortex core, as illustrated in Fig. 1. If the crosssectional area of the vortex tube is assumed to remain constant along its length, then together with the assumption of incompressibility the v_{twist} velocity would need to be constant on each vortex. The helicity conservation would then fix the time dependence of v_{twist}.
We can now see that if the total tangential velocity is zero everywhere on the vortex, we recover Eq. (13) for the internal twist angle that was obtained by using the Seifert frame for superfluid vortex filaments. Since the vorticity of a superfluid vortex does not have an azimuthal component, superfluid vortices do not have an additional intrinsic degree of freedom that can be ascribed to classical vortices. Therefore, in the Seifert frame, the helicity of a superfluid vortex is always zero. In contrast, N is determined by the structure of the vorticity field within the core of a classical vortex and, as such, the helicity is not necessarily the same as for a superfluid vortex.
By assuming that the helicity would remain zero also for the classical case, and that the twist velocity remains constant along the filament as required by incompressibility, the internal twist angle for vortex i is obtained using the following equation:
Here denotes the length of vortex i. If we want that the helicity is simply given by linking, one should only replace v_{BS} in Eq. (16) with the velocity caused by vortex i alone, i.e., set L_{ij} = 0.
Both Eqs (13) and (16) give zero helicity and the same value for the total twist T. The difference appears only in the local value of the internal twist angle, i.e., the frame in the classical case is generally different from the Seifert case since it is associated with the structure of the vorticity within the core.
Straight vortex with a Kelvin wave
Initially, we will focus on idealised vortex configurations to elucidate the different properties of helicity in order to facilitate our understanding of how helicity behaves in more realistic situations. A straight vortex with only an azimuthal velocity field around its core has zero helicity. We will, therefore, consider perturbations on an otherwise straight vortex in the form of a helical Kelvin wave with amplitude A, i.e.:
The last equation relates z to the arclength ξ. The unit tangent , principal normal , and binormal are then given by
In this case, the local torsion is constant and equal to , as would be expected for a simple helix. The value for the writhe (which can be computed as described in ref. 25) and the torsion (per unit period of λ = 2π/k) are
The value for the writhe implies that the tangential component of the BiotSavart velocity is constant and given by
Using Eq. (13), the direction of the constant phase is given by
Consequently, for helicity to be zero, the internal part of the twist becomes T_{tw} = −1 (per period). We note that the formulation given by Eq. (16), obtained by using the (constant) twist velocity, gives exactly the same value for the internal twist angle as the formulation using the Seifert frame, Eq. (13). By setting the integration constant θ_{0} = π, the spanwise vector becomes
Therefore, for small amplitudes . Moreover, we see that N does not rotate around the zaxis, as shown in panes a) and c) of Fig. 1, where the helicity is zero. The internal twist originates from the rotation of the normal and binormal vectors relative to the spanwise vector.
Vortex ring with a Kelvin wave
Next, we consider a superfluid vortex ring with one Kelvin mode, m, where the configuration is given by
Here ϕ is the azimuthal angle of a cylindrical coordinate system, R is the ring radius, and A is the amplitude of the Kelvin wave. As the amplitude of the Kelvin wave is increased from zero, the standard BiotSavart velocity v_{BS} produces a nonzero component along the vortex tangent. On the other hand, if there are no other vortices threading the vortex ring, the helicity should remain zero for any Kelvin wave amplitude.
However, if we evaluate the local torsion and the writhe we notice that at small amplitudes they exactly cancel each other. This implies that the internal twist T_{tw} as defined must be equal to zero in order for the helicity to remain zero. However, at a critical amplitude of A_{c} = R/(m^{2} + 1), m separate inflection points appear where the curvature vanishes and the torsion part of the twist jumps by m due to divergences in the local torsion. [Note that in the article by Moffatt and Ricca^{22} the critical amplitude was stated to be A_{c} = R/m^{2} which seems to be valid only for large m]. This behaviour is illustrated in Fig. 2a, where we have plotted the writhe and torsion part of the helicity, plus their sum as a function of the Kelvin wave amplitude. This key observation shows that, for A > A_{c}, the internal twist must give rise to a compensating contribution of T_{tw} = −m to conserve helicity. These observations are also consistent with the predictions of Moffat and Ricca^{22} obtained for a classical vortex tube.
To determine the internal twist angle (up to a constant), and, therefore, also the spanwise vector, N, we can either use Eq. (13) for the direction of the constant phase, or alternatively use Eq. (16) for the classical case. Figure 2b illustrates the internal twist angle θ when using the Seifert frame, Eq. (13), for the case of m = 3 at various Kelvin wave amplitudes. At the critical amplitude, A_{c}, the angle θ has a jump of π at the azimuthal locations , i = 1, …, m. This jump compensates the jump of −π in the normal and binormal around the tangent, thus ensuring that the N vector varies smoothly as we move along the length of the vortex. The behaviour of the unit vectors and N is illustrated in Fig. 3 for few different Kelvin wave amplitudes and with m = 3. We note that in this case, the normal and binormal vectors make three complete rotations around the tangent only for amplitudes above A_{c}.
Numerical examples for single vortices
We will now focus on how the different contributions to helicity vary in time under a dynamical evolution of a vortex filament. In particular, we will be interested in an example where the vortex passes through an inflection point as it evolves. One example where inflection points appear is a breather solution^{26}. However, in that case the inflection points appear in pairs such that the torsion term T_{tors} is not effected and subsequently no changes occur in T_{tw}. If mutual friction is added into the equations of motion (see Methods), the amplitudes of the Kelvin waves decay with time. This is also accompanied by a decay of internal twist that can be clearly seen in our simulations. An example of a simulation where mutual friction is included for an initial helical vortex ring is presented in the inset of Fig. 4a. The results illustrate how the torsion part of the twist suddenly drops by 3 when the configuration passes through three inflection points. At the same time the internal twist that has an initial value of −3 jumps to zero such that the helicity remains zero.
We have also modelled the dynamics of a trefoil knot at zero temperature. The main panel of Fig. 4a illustrates the behaviour of the writhe and torsion, plus their sum, in the case of the trefoil knot where the initial configuration (x, y, and z in mm’s), parametrized by t ∈ [0, 2π), is given by
As for the vortex ring, we observe integer jumps in the torsion even though we are at zero temperature due to the creation of inflection points as can be seen in Fig. 4a. These results demonstrate that the jumps of ±1 in the torsion must be compensated by jumps of in the internal twist in order to conserve the helicity. To ensure numerical accuracy, we have checked that the energy and momentum are conserved to within 0.1 percent throughout these simulations, up to the time of reconnections, which occur at times >60 s.
The behaviour of the spanwise vector N in the Seifert frame and the normal vector during the trefoil knot dynamics is illustrated in Fig. 4b,c. It is clear that following the formation of an inflection point (see Fig. 4c) that the Seifert frame, depicted by the yellow stripe, and the FrenetSerret basis (green stripe) rotate in opposite directions. Therefore, whereas one varies covariantly, the other varies contravariantly which follows from their definitions. It is this property that results in the observed jump in the torsion at inflection points.
Vortex reconnection
The conservation of helicity during vortex reconnections is an interesting topic of its own because in superfluids reconnections of vortex filaments can arise from quantum mechanical effects that are absent in classical fluids. In a microscopic model, such as that given by the GrossPitaevskii equation, they are made possible by the “quantumpressure” term which acts to couple the incompressible and compressible modes of the system. Using the GrossPitaevskii model, the effect of reconnections on helicity has recently been analyzed in several papers^{16,17,18,19,25}.
In the vortex filament model, reconnections must be modelled phenomenologically by using a “cutandpaste” method. Nevertheless, it is instructive to see what happens when we follow the dynamics through a single reconnection. When reconnections are modelled in this way, the calculation of the local torsion, which requires third order derivates of the vortex positions, becomes numerically very challenging and typically the torsion part of the twist cannot be properly determined. The reason is that in a microscopic model, reconnections lead to strong radiation of sound that dissipates energy of high frequency Kelvin waves resulting in wellbehaved dynamics. This physical process is absent in a vortex filament model. In order to reduce the noise when calculating the torsion, we have increased the vortex core size in this simulation to a_{0} = 0.0025 mm, which is of the order of the numerical resolution given by the interpoint separation which varies between 0.005 mm and 0.010 mm. A reconnection is then performed when the vortex separation is smaller than 0.004 mm, provided that the total length decreases. Additionally, we have included a rather large mutual friction, α = 1, in order to smooth out the small scale structures.
Figure 5 illustrates the reconnection of two vortex rings with initial radii of 1 mm, and which are initially linked (in the form of a Hopf link). The leftmost panel of Fig. 5 illustrates the time development of the different helicity components, while the other panels show the behaviour of the normal vector and the spanwise direction when using the Seifert frame. A characteristic feature is that before reconnection, both vortices host one inflection point. Additionally, one may notice that at the instant of reconnection the linking is converted to writhe, which then decays due to mutual friction, as shown more clearly in the inset of Fig. 5a.
Vortex bundle
The above results reveal the consequences of working in the Seifert framing. However, a central question that remains is how would a quasiclassical limit of helicity emerge if we accept that helicity is trivially zero for a single superfluid vortex filament. From our considerations presented in Section Helicity for vortex filaments we note that a classical vortex tube is well approximated by a bundle of vortex filaments that are aligned to the local vorticity field within the core of a classical vortex. In fact, such a quasiclassical limit of vorticity in superfluids has already been invoked to explain the measured Kolmogorov spectrum in superfluid turbulence^{27}.
The bundles (or polarized discrete vortices) are created by stirring the superfluid. Remarkably, once formed, these polarized vortex bundles behave as coherent structures and can persist as has been illustrated from numerical simulations in ref. 28. Accepting that such coherent vortex bundles give rise to a quasiclassical vorticity field, it follows that the classical analogue of vorticity is defined by: 1) how the vortex lines within a vortex bundle twist around the centreline of the bundle; 2) how the centreline of the bundle writhes. So the quasiclassical notion of helicity is not tied to the Seifert frame but emerges from the linking of vortex lines within the bundle. This is consistent with our observation in Section Helicity for vortex filaments that for a classical vortex tube, the twist is determined by the vorticity within the core and is unrelated to the Seifert frame. This implies that aside from the microscopic attributes of helicity for a single vortex filament, the quasiclassical limit should give rise to an emergent helicity conservation when the bundle evolves in the absence of reconnections.
To illustrate this behaviour, we have performed a numerical simulation of a bundle consisting of seven vortex rings perturbed with Kelvin waves and twisted 3 times around the bundle centreline, as shown in Fig. 6a. Details for of how the intial configuration was set up can be found in the Methods section. Upon integrating this configuration with the vortex filament model, we evaluated how the centreline writhe and the twist varied with time as shown in Fig. 7. As can be seen, although the writhe and twist vary, their sum remains essentially constant. The jumps in the centreline torsion are again due to inflections points in the centreline and are compensated by the internal twist. The noise in the total helicity is partly caused by the finite resolution which softens the jumps in the torsion but also because the bundle is loosing its coherence at later times. For example, in Fig. 6b, the different vortices remain as singlevalued functions of the azimuthal angle. However, in Fig. 6c, steepening of the Kelvin waves on individual vortices destroys the coherent alignment of the vortices. Despite this, we note that since the helicity is approximately conserved and that the twist was evaluated from the rotation of the vortices within the bundle about the centreline, as described in the Methods section, our results provide direct evidence of the emergence of a nontrivial quasiclassical helicity as an invariant of coherent vortex bundles.
Conclusions
When decomposing helicity into its constituent contributions, linking number, writhe, torsion, and internal twist, we find that the first three are completely prescribed by the instantaneous configuration of a vortex filament, whereas internal twist requires a spanwise vector to be defined. The sum of the first three contributions is an integer value and varies only when inflection points appear. In that regard, the torsion contribution to the helicity should always be retained when evaluating the helicity of a superfluid vortex which would otherwise never remain conserved under deformations of the vortex (even those that do not form inflection points). This is consistent with the results found in ref. 25 where it was apparent that helicity was not conserved when only the writhe contribution was retained for a knotted vortex. A method that allows helicity to be evaluated directly from the wavefunction of the GrossPitaevskii model of a superfluid has recently been presented in ref. 19. We note that the expression presented there reduces to the linking and writhe contributions only and, therefore, the observations made above would also be expected to apply to the definition of the helicity presented in that work. The term centreline helicity is sometimes invoked to refer to only the linking and writhe contributions as in ref. 25. However, in other works, the total torsion is also included in the definition of centreline helicity as in ref. 29. In our view, it would seem more appropriate to include the total torsion in the definition of the centreline helicity since it is a quantity that is fully determined by the instantaneous configuration of the vortex and has the desirable property that it is an integral quantity although not necessarily conserved under a diffeomorphism that produces an inflection point.
At zero temperature, the LIA (Localized Induction Approximation), where only the local term of Eq. (26) is retained, possesses an infinite number of invariants, one of them being the integral of the torsion over the vortex length. This conservation of the torsion requires that inflection points appear in pairs, one contributing a change of +1 to T_{tors} and the other giving a change of −1. In other words the internal twist remains constant during the LIA dynamics. Inclusion of the internal twist restores helicity conservation even when inflection points are formed. Defining the twist using the direction of the phase precludes the possibility of having an isolated twisted vortex ring. The phase of a twisted circular superfluid vortex would have a singularity at the centre. This is in contrast to the conventional definition of the twist. A circular vortex tube may be twisted, as illustrated by our bundle calculations where the tube was modeled by using seven vortices. The twisting of vorticity lines inside the tube induces a velocity along the vortex, but does not change the velocity potential outside the vortex tube.
Whether the Seifert framing for superfluid vortices could be justified from first principles is left as an open question in this work. However, it appears to be a reasonable choice from at least three physical points. Firstly, it provides an unambiguous means to define the spanwise vector N that remains welldefined throughout the dynamics and in doing so it restores many of the characteristics of helicity that are known to hold for vortices in classical fluids. Secondly, it ensures helicity is conserved throughout the dynamics for superfluids even during reconnection events even though the different contributions would change to reflect the changing topology of the vortex lines. A consequence of the Seifert framing is that this choice connects the linking with the internal twist. For example, two vortex rings which separately have zero twist, become twisted if linked (e.g. a Hopf link). Thirdly and most significantly, we have shown how a nontrivial quasiclassical limit of helicity can emerge that is independent of the Seifert framing.
Methods
Dynamics with the filament model
The dynamics of quantized vortices is typically modelled with the filament model^{30} such that the vortices are considered as thin tubes with cylindrically symmetric cores where the circulation generates a classical Magnus force. Given the extremely small vortex core, we may ignore the small effective mass of the vortex although in general this effect can become more important at very low temperatures and on scales comparable to the core size. At finite temperatures, one additionally needs to consider dissipation due to the mutual friction that couples the superfluid and normal components together. Setting the sum of the Magnus and mutual friction forces equal to zero results in the following equation of motion for the vortex lines:
Here v_{n} corresponds to the normal fluid velocity while v_{s} corresponds to the superfluid velocity which is given by v_{s} = v_{BS} + v_{Ex} where v_{Ex} corresponds to some externally imposed irrotational superflow which we set equal to zero. Both the normal (v_{n}) and superfluid (v_{s}) velocities are evaluated at the vortex (centreline), s, whereas derivatives are evaluated with respect to the arclength, such that corresponds to the unit tangent vector. The two parameters α and α′ represent mutual friction coefficients that depend on temperature and pressure. The effect of the corresponding terms is to damp out excitations such as Kelvin waves on the vortices. For calculations at finite temperature we also ignore the coupling from superfluid vortices on the normal component and take v_{n} = 0. This approximation is especially suitable in superfluid ^{3}He where the viscosity of the normal component is high.
Since we need to evaluate the superfluid velocity along the vortex centreline, we must introduce a cutoff to avoid the singularities in the superfluid velocity field arising from the divergent terms appearing in Eq. (7) for v_{BS}. This is accomplished by introducing a finite core size cutoff. This way the singularity in the azimuthal component of the velocity (as mentioned above, the tangential component of v_{BS} is regular) can be avoided and the BiotSavart velocity at a vortex point becomes
Here the derivates are again with respect to arclength ξ, and the integral omits the short segments l_{±} around the point s. The first term is called the local term and it produces a velocity along the binormal with amplitude proportional to local curvature c = s″. The coefficient a_{0} is the vortex core size and the βparameter is related to the core structure, being 1/4 for a solid rotating core model (Rankine vortex) and 1/2 for a hollow core vortex. It is tuned such that the local term gives the same velocity for a vortex ring (or its local segment) as that of a classical vortex ring with a similar core structure. The approximation made for the local term is valid when .
Twist contribution for the vortex bundle
For the initial configuration we used a bundle of seven vortices where the centremost vortex, which initially is also the centreline, had a shape of the ring with a Kelvinwave, Eq. (23). We set R = 1 mm, and A = 0.1 mm. The twist of the bundle was achieved by twisting the 6 outermost vortices by 3 times (corresponding to an angle of 6π) with respect to the untwisted bundle, which can be obtained by setting the 6 outermost vortices at directions determined by the constant phase directions of 0, 2π/6, …, 10π/6, of the centre vortex (calculated when omitting the effect of the outer vortices). The twisting angle with respect to this untwisted configuration was chosen to depend linearly on the arclength along the centreline. The distance of the outermost vortices from the centre vortex was 0.1 mm. Around 7000 points where used to discretise the vortices. These parameters were chosen primarily due to constraints set by the numerics.
During the time evolution of the vortex bundle the centreline was determined by averaging over the azimuthal locations of the seven different vortices. When deformations from a circle are not too large, this approximation is suitable. When evaluating the internal twist for the bundle, the direction of the different vortices with respect to the SerretFrenet basis of the centreline was determined. In other words, the angle, θ, appearing in Eq. (4), was calculated for each vortex as a function of the length along the centreline by determining the crossing point of each vortex on the plane determined by and .
As long as the bundle remains coherent, the twist of the different vortices remains the same. The only exception was the centremost vortex, which initially determined the centreline. Because the centremost vortex may be very close to the centreline, the twist was determined using only the initially six outermost vortices.
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How to cite this article: Hänninen, R. et al. Helicity within the vortex filament model. Sci. Rep. 6, 37571; doi: 10.1038/srep37571 (2016).
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Acknowledgements
R.H. and N.H. acknowledge support from the Academy of Finland (LTQ CoE Grant, and Grants 218211 & 292766). H.S. acknowledges support for a Research Fellowship from the Leverhulme Trust under Grant R201540. We thank especially J. Karimäki, M. Krusius, R. Ricca, G.E. Volovik for fruitful discussions, comments and improvements to the paper. We also like to thank CSC  IT Center for Science, Ltd., for the allocation of computational resources.
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R.H. conducted the simulations and wrote the first draft of the manuscript. Some analysis tools where written by N.H. All authors contributed to the theory development and participated in the writing and review process of the manuscript.
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Hänninen, R., Hietala, N. & Salman, H. Helicity within the vortex filament model. Sci Rep 6, 37571 (2016). https://doi.org/10.1038/srep37571
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