Abstract
Freesurface vortices have long been studied to develop an understanding of similar rotating flow phenomena observed in nature and technology. However, a complete description of its turbulent threedimensional flow field still remains elusive. In contrast, the related TaylorCouette flow system has been well explicated which classically exhibits successive instability phases manifested in socalled Taylor vortices. In this study, observations made on the turbulent freesurface vortex revealed distinguishable, timedependent “Taylorlike” vortices in the secondary flow field similar to the TaylorCouette flow system. The observations were enabled by an original application of 2D ultrasonic Doppler velocity profiling complemented with laser induced fluorescence dye observations. Additional confirmation was provided by threedimensional numerical simulations. Using Rayleigh’s stability criterion, we analytically show that a wall bounded freesurface vortex can indeed become unstable due to a centrifugal driving force in a similar manner to the TaylorCouette flow. Consequently, it is proposed that the freesurface vortex can be treated analogously to the TaylorCouette flow permitting advanced conclusions to be drawn on its flow structure and the various states of freesurface vortex flow stability.
Introduction
Concentrated vortices are fascinating yet highly complicated flow phenomena which have deservedly been studied for centuries in the contexts of nature and technology^{1,2,3,4}. The classic, freesurface draining vortex, or the socalled “bathtub” vortex is among the most captivating of the families of vortex flows owing to the highly familiar yet unique depression of the freesurface accompanied by rotating surface ripples and a distinct appearance of “swirl”. However, beneath the surface and hidden to the eye of the observer is an intricate assembly of space and time dependent flow processes which still lack complete scientific elucidation^{5}.
In general, freesurface vortices (FSVs) result from natural or artificial field circulation Γ_{∞} conditions generating a strong primary tangential velocity field v_{ θ }(r) characterised by turbulence through the vortex Reynolds number Re_{Γ} = Γ_{ r }/ν and rotational strength by the circulation number N_{Γ} = dΓ_{∞}/Q. They can exist as either a ‘strong’ full air core or a ‘weak’ collapsed air core type which transition as a freesurface instability at the critical submergence S_{ c }^{5,6,7,8}. The primary tangential velocity field v_{ θ }(r)in the freesurface vortex is superimposed on a more complex secondary flow field comprising the radial v_{ r } and axial v_{ z } velocity field which are responsible for ensuring continuity of flow Q through the system^{9}. In two seminal studies undertaken independently on turbulent vortices by Anwar^{10} and Daggett and Keulegan^{9} it was discovered that the bulk of radial and axial flows were strongly localised to thin layers close to the base of the vortex, the freesurface and the air core region respectively and both studies suggested that it was the flow Q “that provides energy to maintain an open vortex”^{9}. This was pivotal in providing an understanding of how full air core vortices maintain stability. Andersen et al.^{5,6}, in their contribution on the “anatomy of the bathtub vortex” also scrutinised the secondary flow field and attempted to decipher its composition, albeit for the weak laminar vortex flow. In their study^{5,6} they observed similar localised wellstructured flow layers at low Reynolds number Re_{Γ} = 3 × 10^{3}. At higher Reynolds number flows (Re_{Γ} = 7 × 10^{4}), Echávez & McCann^{11} also noted similar flow layers at the boundaries and observed the appearance of well defined “hoodlike” structures in the secondary flow field sub_{}surface depths. When dealing with turbulent vortices at Re_{Γ} = 8 × 10^{5}, Anwar^{10} commented on the observation of aluminium particles suspended in the flow being drafted upwards near the core and thrown radially outwards indicating more intricate spatiotemporal flow behaviour at play in this subsurface region. He also stated^{12} that the tangential velocity distribution v_{ θ }(r)differs from the laminar case due to the onset of turbulence triggered by the localised instability of curved flow as originally projected by Scorer^{13} who also pointed out that turbulence is attributed to large variations in axial flow in this region. It is clear from this that the turbulent FSV introduces higher degrees of complexity to the secondary flow field that demands a more complete analytical and experiential understanding.
A relative of the FSV in the family of rotating flows is the classic Taylor–Couette flow (TCF) of an incompressible, viscous fluid in the gap between two concentric rotating cylinders of radii r_{ i }, r_{ o } (r_{ o } > r_{ i }) and height l^{14,15,16} as described in Fig. 1a. The control parameters of the system are generally taken^{17} as the radius ratio η = r_{ i }/r_{ o }, the cylinder angular velocity ratio μ = Ω_{ o }/Ω_{ i }, the aspect ratio ζ = l/(r_{ o } − r_{ i }) and the Reynolds number Re defined by the Taylor number by Ta \(=\,{r}_{i}{{{\rm{\Omega }}}_{i}}^{2}{({r}_{o}{r}_{i})}^{3}/{\nu }^{2}\) which drives the flow by shear from the cylinder with an angular velocity of of Ω_{ i }^{18}. The tangential velocity between the cylinders then takes the form of:
where the noslip (shear driven) boundary conditions are:
At small angular velocities of the internal cylinder, the driven flow is laminar and purely azimuthal (the circular Couette flow, CCF). Taylor^{15} recognised that when the angular velocity of the internal cylinder exceeded a critical value, referred to by the critical Taylor number Ta, a primary instability developed whereby the flow became unstable to axisymmetric perturbations and the radial v_{ r } and axial v_{ z } velocity components manifest into steady stacked counter rotating vortices. This threedimensional laminar flow is known as TaylorCouette (TCF) flow and upon further increase of the rotation beyond a series of subsequent critical values, the flow becomes unstable to unaxisymmetric perturbations and azimuthal waves develop on the tori which eventually becomes chaotic leading to a fully turbulent regime^{19}. The TCF problem has also been demonstrated for concentric cylinders with a freesurface^{20,21}. Most notably from this, Dunst^{21} shows using observations of dye on a wide gap (small radius ratio) freesurface Couette flow, that the inertial stability of the flow depends largely on μ describing the momentum generation as a sink or a source. Using Rayleigh’s stability criterion^{22}, Dunst^{21} highlighted that the whole flow field can become unstable with the rotation of only the inner cylinder. In such a case, Dunst^{21} also made observations of strong inwards radial flow at the base of the tank which became weaker in the subsurface region. The inward flow for a TaylorCouette flow was also noted by Ogawa^{23} prior to the formation of turbulence again on small radius ratio configuration. In general, these observations are similar to inward flow bands discussed by Anwar^{10} and Daggett and Keulegan^{9}. In summary, many studies have been performed on this topic and the TaylorCouette flow system has remained an ideal model to study instabilities, nonlinear behaviour and transitions to turbulence in fluid flows over the past number of decades^{19,20,24,25,26,27,28,29,30,31,32,33}.
From both flow systems (the TCF and the FSV) it is interesting to point out that for the case of a fixed outer boundary, the velocity field decreases monotonically in a radial direction outwards^{34}. In the following study, implementation of analytical, experimental and numerical analysis of the turbulent freesurface vortex chamber reveals a number of further compelling similarities between both flow systems. Most notably, experimental and numerical analysis confirms the existence of ‘Taylorlike’ vortices residing in the secondary flow field of the FSV which are proposed to be triggered by a centrifugal driving force. The formulated analogue between the TCF and the FSV systems differs mainly by energy transfer where the former is mechanical driven and the latter is driven by continuity of flow. However, in order to override this contrast, one simply has to visualise the air core of the FSV as a ‘virtual inner cylinder’ to perceive the reverse effect. We show that through this analogue, the instability mechanisms are indeed the same by considering Rayleigh’s stability criterion. As will be discussed, this discovery and descriptive analogue to the TaylorCouette flow system has significant implications for a fuller understanding of turbulent freesurface vortex flow behaviour and stability.
Results
Instability mechanisms in strong freesurface vortices
Considering th vortex flow problem as outlined in (Fig. 1b) with no outer boundary. Using the quasicylindrical approach for an ideal fluid it is easy to infer from the radial momentum equation that v_{θ(FSV)} = V(r) = Γ_{∞}/2πr as shown by others^{34} where Γ_{∞} is the constant circulation field. To compare generally with the circularCouette flow (CCF), if we remove the external cylinder (or boundary) in this problem by setting r_{ o } → ∞ and thus η → 0 in Equations (1) and (2), the tangential velocity profile then becomes \({v}_{\theta (CCF)}=V(r)=\,{{\rm{\Omega }}}_{i}{{r}_{i}}^{2}/r\), which is mathematically similar to the ideal freesurface vortex primary flow field. In order to extend this analogy, let us next consider the tangential momentum equation of the NavierStokes equations as follows:
which, through the quasicylindrical approximation^{3}, simplifies to:
This linear second order ordinary differential equation is then solved for the vortex flow system with an outer curved boundary to become:
By isolating a radial section of secondary flow field and imposing the boundary conditions of rotation at the air core interface r = r_{ a } (analogous to the rotating inner cylinder of the TCF) and at a stationary or nonstationary curved boundary some radial position r = r_{ o } by v_{ θ }(r = r_{a,o}) = v_{θa,o} = Γ_{ r }/r_{a.o}, the equations for A′ and B′ become:
where Γ_{ r } is the circulation distribution along r, μ_{ v } = v_{ θo }r_{ a }/v_{ θa }r_{ o } and η_{ v } = r_{ a }/r_{ o }. The freesurface vortex velocity field can then be solved to become:
Equation 7, for a stationary boundary μ_{ v }= 0 then becomes
To investigate inertial stability in this case, consider two fluid particles of same mass positioned at r = r_{1} and r = r_{2} in the flow field as shown in Fig. 1f. The combined kinetic energy of both particles sums to:
where L_{1,2} = v_{θ1,2}r_{1,2} is the angular momentum. If under some circumstance or perturbation, both particles were to suddenly swap position, each conserves its angular momentum, and the new combined energy becomes:
Thus, the energy change from E → E_{ new }becomes:
If the swap results in a release of energy \(({\rm{\Delta }}E < 0,\,{{L}_{2}}^{2} < {{L}_{1}}^{2})\), the laminar flow will be unstable to such a perturbation. Thus the Rayleigh criterion^{22} for instability requires that the derivative with respect to r of the square of the angular momentum is less than zero by
By substituting Equation 8 into Equation 12 it is possible to show that the secondary flow field of the FSV with an outer stationary wall can become unstable to axisymmetric perturbations in an analogous manner to the TCF.
For the purpose of investigating the aforementioned analogue further, a strong and steady freesurface vortex flow, using water as the fluid, is generated in a scroll type vortex chamber where the walls follow a logarithmic spiral r_{ p }(θ) = ae^{bθ} centred about a 67 mm discharge as outlined in Fig. 2. A flow Q generated by pumping is conveyed into a baffled channel which creates a steady hydrostatic approach flow depth h in the tangential inlet. Six subcritical steady state approach flow depths were examined (1.38 × 10^{5} ≥ Re_{Γ} ≥ 2.07 × 10^{5}). A full description of the experimental test rig is available in the following methodology section and also in a study performed by Mulligan et al.^{35}.
To facilitate a comparison with the TaylorCouette flow, the variation of vortex flow depth h (to vary the energy of the flow system) ensued various aspect ratios defined by ζ_{ v } = h/(r_{ o }(θ) − r_{ a }). The radius ratio also varied with respect to θ and r_{ a } by η_{ v }(θ, r_{ a }) = r_{ a }/ae^{bθ}. Thus the geometry, and any geometry induced instability mechanisms, must be asymmetric (effects of which will be discussed later). In order to isolate the dependence of the spiral walls, measurements and observations were undertaken at a fixed secondary plane of θ = 45 ° and 225 ° for planar laser induced fluorescence observations and ultrasound Doppler profiling as outlined in Fig. 2 where the inlet is positioned at θ = 0°. To be consistent with the TCF, we also formulate a new variation of the vortex Reynolds number Re_{Γ} to take into account the characteristic radii defined by the gap between the air core and the outer most boundary (r_{ o } − r_{ a }) by:
Global secondary flow field behaviour
Initially, qualitative secondary flow field observations were made using the elements of PLIF (Fig. 2) to provide basic dye advection observations. Figure 2a and b indicates the dominant flow patterns observed in the secondary flow field using PLIF. By injecting a small quantity of Rhodamine B dye at the tank base and at the freesurface, advection layers were observed to develop in both regions which demonstrated radial inflow towards the orifice and downwards axial flow at the vortex core. The results were in line with the observations made by^{9,10}. Additional transport of the dye was observed in an upward axial direction along the chamber walls which conveyed flow to the freesurface and consequently the core region. This revealed a global quasitoroidal flow pattern in the secondary flow field. The system was entitled ‘quasitoroidal’ owing to the fact that the toroidal loop was strictly unclosed due to a transient separation point occurring at some region near the floor or wall as shown in Fig. 2c.
Radial and axial velocity profiles using UDP
In order to provide a detailed quantitative examination of the global secondary flow field at 225 °, velocimetry was performed using UDP and an original flow mapping technique which was a first application of 2D array UDP in freesurface draining vortices. High spatial and temporal resolution v_{ r } and v_{ z } profiles at various z and r positions respectively was achieved using the array configuration of UDP transducers outlined in Fig. 3, which leveraged the approaches of others on TC systems^{19,36,37}. Individual profiles were obtained at 19 ms with an in axis resolution of resolution of 2.5 mm/s. This arrangement also permitted 2D velocity flow maps to be constructed over the secondary flow field. Further information on the UDP configuration is outlined in the following methods section.
Figure 4a displays the quantitative signature of the cellular structures using a spatiotemporal map of the axial velocity distribution for h/d = 2.0 where the axial velocity alternates between the negative downward and upward positive profiles passing through counter rotating zones. The spatiotemporal map indicates that the vortices do not vary significantly within the 0.3 second time frame as indicated by the approximate positive and negative bands determined along the transducer 4 profile (Fig. 3b). Figure 4b highlights the standard deviation of the average velocity profile determined throughout the 0.3 s interval consisting of 16 profiles (19 ms sampling period).
Figure 4c,d,e and f highlights instantaneous axial (transducer 4) and radial (transducer 8) profiles for h/d = 1.5 and 2.0 respectively. Figure 5e and f indicates that there is an outward flow near the tank periphery in both cases whereas near the core the flow can switch between inward (negative velocity) and outward (positive velocity) flows. The vertical position of the horizontal transducer 8 at 11 mm above the base is such that the beam profile is not completely within the bottom flow band outlined in the PLIF experiments. Hence, near the core at a short distance up from the base of approximately 10 to 30 mm there is highlight unsteady, oscillating behaviour. This inward, outward switching of radial velocities developing close to the air core for high depths h/d 1.5 was in line with the observations made by in Fig. 4 and by Anwar^{10} on small suspended particles in the flow field in this region.
For low approach flow depths of h/d ≤ 1, the radial and axial velocity did not reveal cellular flow structures and only highlighted flows residing at the boundaries. Any observations of the flow field above an approach flow depth of h/d = 1.5 (M = 2.22 × 10^{5} and ζ_{ v } = 0.58) exhibited definite unsteady characteristics in the secondary flow field; i.e. the position and magnitude of the vortices varied with time. A prolonged time series for the axial velocity at a subsurface point in space indicated that the flow field was quasiperiodic or chaotically wavy, similar to that described by Takeda^{19} in TaylorCouette flows. Both the core tangential and axial velocities were recorded to be of the order of 1 to 2 m/s whereas, in all cases, the Taylorlike vortices exhibited velocities that were two orders of magnitude smaller than the core velocities at 0.005 to 0.05 m/s. This is very similar to the observations made by Dunst^{21} on a freesurface TaylorCouette flow with a small radius ratio. Dunst^{21} also found a strong inward flow near the bottom and a weak outward flow in the subsurface region indicating that there is a ‘source’ of angular momentum generated. The transition between the inward flow band and the weak outward flow is analogous to the observations made in this region in the FSV using UDP.
Taylorlike vortices
Due to the relative stability of the cellular structures observed in Fig. 4a and b, it was possible to use the transducer array to construct quasiinstantaneous 2D velocity vector maps for various h/d. As shown in Fig. 5a and b, the 2D flow maps confirmed the existence of ‘Taylorlike’ vortices where loosely structured counter rotating cellular structures can be observed. The loosely structured features may have been a result of the small radius ratio 0.152 ≥ η_{ v } ≥ 0.090 resulting in a lower instability threshold together with the large Reynolds number in the flow field of the order of 10^{5}. Residual artificial perturbations introduced from the inlet conditions may also have contributed to their loosely structured appearance. No cells were observed for h/d = 0.5 (ζ_{ v } = 0.2); one or two cells were observed when h/d ≥ 1.0 (ζ_{ v } ≥ 0.4) and two or three cells were observable when h/d ≥ 3.0 (ζ_{ v } ≥ 1.0) which describes that the number of cells increase with aspect ratio ζ_{ v } similar to Watanabe and Toya’s^{20} observations on small aspect ratio freesurface TCFs.
A final clarification of the composition of the secondary flow field was achieved through threedimensional transient numerical modelling using Reynolds stress turbulence modelling. The simulation was performed on a model with a larger radius ratio 0.09 ≥ η_{ v } ≥ 0.16 for approach flows of h/d = 1.0, 2.5 and 3.5. Figure 6a–c presents instantaneous streamlines and vorticity contours generated on the secondary flow field. Similar to Figs 2 and 4, the secondary flow field was found to be composed of strong advection layers forming at the base of the tank, the freesurface, vessel walls and orifice with superimposed cellular structures. The cellular structures originated at the tangential inlet once the fluid underwent streamline curvature and appeared to wrap and spiral around the vortex core terminating close to the bottom outlet. For the low approach flow depths of h/d = 1.0 the flow field appeared to retain a rotational threedimensional laminar flow which often bifurcated to two parallel cells (Fig. 6a) before merging again into a single cell. At h/d = 2.0 (ζ_{ v } = 0.95), the flow field comprised of two wellstructured stable cells as shown in Fig. 6b. At h/d = 3.5 (ζ_{ v } = 1.637) three cells were apparent in the flow field and the Taylorvortices exhibited wavy patterns. Figure 6e and f highlights the variation of the v_{ z } with time t at various axial positions z/h along the radial position r = 0.1 m. As the approach flow depth is increased from h/d = 1.5 to 3.5, the v_{ z } time series varies from a lightly transient (wavy) (Fig. 6e) to a state to highly transient chaotic state (Fig. 6f).
Discussion
We have shown that strong freesurface vortices exhibit strong similarities to the TaylorCouette flow system through the flow mechanics of the primary and secondary flow field and observations of “Taylorlike” vortices. The various levels of unsteadiness could be lightly classified into various modes of instability similar to the TC flow up to the chaotic wavy mode. However, the exact instability thresholds of each qualitatively observed feature is still up for question. Table 1 provides a summary of the chief analogous features between both flow systems as derived from and observed within this study.
The primary difference between the freesurface vortex and TaylorCouette flow lies in the process of energy transfer. In the TCF, mechanical energy is introduced by the rotating inner and outer cylinders that drive the flow via shear and momentum transfer between fluid layers. In major contrast to this, the freesurface vortex flow system behaves in reverse, where the central core derives rotational energy from shear driven circulation field derived from a continuity of flow entering the domain as described by Anwar^{10} and Daggett and Keulegan^{9}. In order to formulate a more complete description, developing on studies from others^{9,10} we propose that it is the global quasitoroidal flow process in the secondary flow field that provides the discharge, and thus, the energy to maintain the vortex (i.e. to bring in new energy to replace that lost to viscosity or turbulence). Thus, this energy from a continuity of flow is analogous to energy introduced by mechanical rotation in the TCF. This hypothesis has significant implications in developing a more unified understanding of the dynamics of the secondary flow field in both strong and weak turbulent freesurface vortex flows as is discussed next.
Despite the dissimilarity in the energy induction process, the freesurface vortex can be treated analogously as a TaylorCouette flow by visualising the vortex air core as a ‘virtual cylinder’. That is to say, for this analogy to be valid we are not obliged to visualise an air core, and similarly the fluid flowing inwards at the boundaries may be supposed to be removed, as its energy maintains the rotation of the ‘virtual inner cylinder’. The analogue was coined in this study as the ‘Analogous TaylorCouette’ flow insofar that, as the energy is increased due to inflow in the freesurface vortex, the air core (or virtual cylinder) narrows and increases in velocity resulting in the generation of rotational instabilities in the secondary flow field in an analogous manner to the TaylorCouette system. The unstable driving force in both flow systems is then a centrifugal one which is to be balanced by the pressure gradient for the flow to remain stable. Thus in the freesurface vortex, the secondary flow field primary instability is developed when a fluid particle is perturbed from its initial position in, say an outward radial direction, beyond the point where the local restoring force due to the pressure gradient is slightly less than the outward inertia of the particle, resulting in the particle continuing to move outwards. Vice versa, a fluid particle perturbed inward will continue inwards and mass conservation will ensure toroidal cell development as shown in Fig. 1f.
However, according to the Rayleigh stability criteria, the secondary flow field can only become unstable when it is contained between an outer wall. As applied to the unbounded case of Fig. 1b where r_{ o } → ∞ and η_{ v } → 0(i.e. the case of infinite curvature) it is easy to deduce from Equations 7 and 8 that the primary flow field is fully irrotational and the flow is stable. The same effect can theoretically occur when you have a bounded freesurface vortex flow where the air core radius r_{ a } → 0 (i.e. the vortex flow approaches the critical submergence depth S_{ c }). However, since azimuthal shear instabilities (which occur for high core velocities) are also associated with a decrease in azimuthal circulation, centrifugal instabilities are likely to render the flow unstable in each case similar to the TaylorCouette flow^{38}. Furthermore, for weak vortices when h ≥ S_{ c }, Gallaire and Chomaz^{38} describe how a centrifugal instability can occur across the Rankine vortex tangential velocity distribution. It is also important to point out that the strong axial downward flow at the core, combined with the fixed boundaries of the base and wall, also renders the problem analogous to a cavity driven flow^{39}. Therefore, instabilities due to axial motion have also to be considered to evaluate the nature of threedimensional, anisotropic turbulence also including azimuthal shear instabilities^{40}. As discussed previously, although the primary flow field is taken to be largely axisymmetric, the secondary vortex instabilities are likely to be asymmetric due to the asymmetry of the approach flow geometry in the current case (r_{ o } ≥ ae^{bθ}), thus, the critical instability threshold varies as one circumferentially spans the system. It is also worth noting that the current analogue may be extended other variations of the TCF system which introduce axial effects (i.e. Spiral—Couette and Spiral—Poiseuille flows^{40}) which may also help describe the formation of asymmetric Taylorlike vortices. The extension of the analogue to consider Spiral—Couette and Spiral—Poiseuille flows^{40} would no doubt be an interesting study.
In more general terms, it is hypothesised that the primary instability of “Taylorlike” vortex behaviour aids the flow system in avoiding chaos in the distribution of flow and energy from the inlet to the outlet regions of the domain while maintaining primary field rotation and an ‘open vortex’. This is inferred from the streamlines originating near the cells shown in Fig. 6 which appear to supply flow to the boundaries and subsequently to the outlet. The Taylorlike secondary vortices were observed to asymmetrically ‘wrap’ around the primary vortex core (or primary vortex line).In general, the cellular wrapping behaviour is close in appearance to the spatiotemporal processes described by Chanaud^{41} on observations of oscillatory motion in the breakdown of swirling flows. Given this, it is wellknown that as the approach flow depth (or system energy) is increased beyond the critical depth, the vortex collapses to form a dimple and the velocity distribution follows a Rankine distribution^{1,7}. To the best of our knowledge, there has been no fluid mechanical description for the role of the secondary flow field during this critical transition, nor a description for the decay according to a Rankine distribution besides the fact that turbulence plays a significant role^{34,42}. A possible explanation may lie in the concept of the TaylorCouette analogy where, as the modes transition from a chaotic wavy to a turbulent flow regime similar to the turbulent Taylorvortices^{19,43}, the combination of centrifugal axial and shear instabilities may, in turn, lead to breakdown and highly anisotropic turbulent flow conditions. There is also a nexus between this line of thinking and the vortex eddy viscosity concept introduced by Anwar^{10} and Einstein and Li^{34}. In these articles, the authors discuss vortex stability on the basis of turbulent momentum transfer without providing a complete description of the origin of this turbulence.
Describing dynamic systems analogously is not a new topic in fluid and particle mechanics. A classic example is the strong similarity between the TaylorCouette flow and the RayleighBenard Convection^{17} system first noted by Rayleigh where he published work on the dynamics of rotating fluids^{22} and convection^{44}. The analogy between the stability of rotating flows and the stability of stratified flows was also analysed by others^{17,45,46,47,48}. Strong analogues have also been identified in an interdisciplinary context where Conway et al.^{49} demonstrated experimentally that granular material flows generate vortices consistent with the TaylorCouette flow in fluids.
Much of meteorology^{50} and astronomy^{31} depends ultimately upon the dynamics of revolving fluids. As stated by Rayleigh, it is therefore desirable to formulate conclusions from “simple approaches within our reach in the hope that they assist our judgement when an exact analysis or observation is impractical”^{22}. For that reason, many studies^{51,52} have considered the TaylorCouette flow as a model to extend to complex astrophysical processes. For example, the instability of viscoelastic TaylorCouette flow was found to be directly analogous to the magnetorotational instability in astrophysical magnetohydrodynamics by Ogilvie and Potter^{53} and further studied by Altmeyer et al.^{54}. Perhaps, freesurface vortices, due to their gravitational inflow and outflow properties (absent in the TaylorCouette flow) together with secondary flow rotational instabilities, may provide further insight into the behaviour of large meteorological systems^{16,54,55,56} or flows on a grander cosmological scale such as black hole accretion disk dynamics^{57}. Jones^{58} speculates that the galactic structure may be maintained by an inflow of stars and gas as they fall into the black hole; directly analogous with how a freesurface vortex is maintained^{9,10}. This would not be the first time that ‘kitchen sink cosmology’ is considered to offer a model for astrophysical systems on a tabletop scale^{58,59,60}. A wellplanned Analogous TaylorCouette system, with consideration for a proper fluid medium may provide an insightful system representation.
Currently, the article gives rise to many unanswered questions such as the magnitude of the critical thresholds, the effects of symmetric boundaries, varying gap width and the effects at the critical submergence. To fully realise the potential of the Analogous TaylorCouette approach, it will certainly be necessary to perform careful systematic experimental studies on the secondary flow field to determine various values of the M parameter through various geometries, particularly at the onset of the critical submergence. We hope to contribute significantly to progress in this regard in future publications.
Methods
Hydraulic test rig and physical models
Details of the test configuration used in this article are presented schematically in the study of Mulligan et al.^{35}. The physical model employed in the experimental study was constructed from 6 mm transparent acrylic and had an orifice diameter of d = 0.067 m, inlet width of b = 0.067 m and an inlet radius of r_{ in } = 0.207 m corresponding to an approach flow geometric factor α = 3.129. The walls scrolled inwards according to the logarithmic spiral r_{ p }(θ) = 0.24e^{−0.057θ}. The test geometries were mounted in a 0.85 × 0.95 m tank which was 0.5 m deep. The tank contained a centrally positioned 0.1 m orifice and rested on a platform over the storage reservoir. A 0.15 m high chamber was used to allow a void to permit the free discharge of flow from the orifice and to give ample space for UDP measurement on the tank underside. The model discharged the test flow to the drop shaft which transferred the flow to the lower storage tank.
The inlet to the test models comprised a 0.065 m bell mouth pipe entrance, 0.14 m perforated plates and honeycomb flow straighteners which homogenised the incoming velocity profile. Water was circulated through the system by a centrifugal pump (flow rate of 0 to 3.5 l/s) and was monitored using a magnetic flow meter (BMeters, Italy) and regulated using two valves. The system monitoring delivered an accuracy corresponding to maximum error bars for intake Froude and radial Reynolds numbers of Fd = ± 0.019 and Rr = ±34, respectively. Approach flow depths h were expressed as a ratio of the constant orifice diameter d = 67 mm by h/d. Tests were performed for 6 approach flow depths corresponding to h/d = 0.5, 1.0, 1.5, 2.0, 2.5 and 3.0. This resulted in an experimental range of vortex Reynolds number Re_{Γ} = 1.38 × 10^{5} to 2.07 × 10^{5} and circulation numbers N_{Γ} = 5.82 to 31.03.
Laser induced fluorescence
A visual observation of the global secondary flow field was achieved using planar laserinduced fluorescence (PLIF). PLIF is an optical flow visualisation technique used to observe the advection and diffusion of a fluorescent dye in the flow. The PLIF process is outlined in Fig. 2. In this application, a 532 nm Nd:YAG laser (Spectron SL404) was used in conjunction with Rhodamine B fluorescein which fluoresces at a wavelength λ = 590 nm wavelength (yellow) under the absorption λ = 532 nm light. The laser emits a 6 mm diameter beam profile which was passed through light sheet optics to generate a 2 mm thick, vertically orientated diverging laser light sheet which was directed to highlight the z − r plane residing at the centre of the vortex. A small quantity of Rhodamine dye was injected at (a) the tank base and at (b) the freesurface at the inlet channel and (c) at the chamber walls and a highspeed camera, positioned perpendicular to the light sheet arrangement, observed the advection mechanisms of the dye. The light sheet and transport of the fluorescein in each observation was imaged at a fixed pulse repetition and frame rate of 30 Hz.
Ultrasonic doppler profiling
An original application of the Ultrasound Doppler Velocity Profile method (UDP method) was developed for analysing the secondary flow field in the freesurface vortex. The UDP principle utilises both echography and the Doppler Effect to respectively determine the position and velocity of a particle along an ultrasonic beam profile and is described in detail by the pioneer of the method, Takeda^{36,37,61}. In our approach, we adopted a twodimensional (2D) flow mapping principle by establishing a 7 × 7 array of ultrasonic transducers along the r − z plane of the vortex to ascertain 2D velocity vectors for a semicross section of the secondary flow field. The transducers could be placed at minimum and maximum centres of 25 mm along the horizontal (r − axis vertical transducers) and 22 mm along the vertical (z–axis horizontal transducers) as highlighted in Fig. 3. A total of 277 samples (channels) were achieved along each profile. A transmitting frequency of 4 MHz was used together with 4 cycles per pulse resulting in a minimum measurable channel width of 0.74 mm and the distance between channels was 0.74 mm. A pulse repetition frequency of 3.52 kHz was used resulting in an inaxis velocity resolution of 2.545 mm/s. Due to an ample concentration of seed particles available in the fluid (10 micron hollow glass spheres), a number of repetitions N_{rep} = 32 sufficed resulting in a time resolution of 9 ms. The transducers were multiplexed in a diagonal fashion using the following trigger sequence with reference to Fig. 3 (S_{ t } = 1–8, 2–9, 3–10, 4–11, 5–12, 6–13, 7–14). 40 flow maps were obtained for each test over a duration of 224 seconds. The 2D velocity fields were smoothed using kriging interpolation and post processed using ParaView. The UDP system was supplied by MetFlow SA (Lausanne, Switzerland).
Threedimensional numerical modelling using multiphase reynolds stress modelling
Numerical modelling was performed using the commercial CFD software ANSYS CFX (V14.5) which uses a hybrid finiteelement/finitevolume (finite element based finite volume method) approach to discretising the NavierStokes equations. Global conservation is satisfied by enforcing local conservation over the control volumes. The finite element approach is used to determine various surface fluxes and source terms within each element. Advection fluxes are evaluated using a highresolution scheme that is secondorder accurate and bounded. The two phase fluid domain was modelled using a homogeneous EulerianEulerian multiphase flow model assuming that interphase momentum transfer is negligible. This was valid for the current test case where the phases were completely stratified and the interface was well defined. In the homogenous approach, both phases are treated as interpenetrating continua parted by a welldefined interface and share a common velocity, pressure and turbulence field.
The Unsteady Reynolds Averaged NavierStokes (URANS) equations were modelled using the 2^{nd} order Baseline (BSL) Reynolds stress model (RSM) which involved solving an equation for transport of the individual Reynolds stress components. Modelling the exact production term and inherent modelling of stress anisotropies theoretically render the Reynolds stress models more suited to complex flows by naturally including the effects of streamline curvature and sudden changes in strain rate. The flow domain was spatially discretised using solution independent, quasistructured mesh arrangement comprising of 2.96 × 10^{6} elements. In order to model the boundary layer accurately 1 < y + < 6 was enforced across the domain. The boundary condition configuration that was chosen which assigned a mass flow at the inlet and a static pressure condition at the outlet with noslip boundary condition assigned to the chamber walls. The physical model arrangement analysed possessed an orifice diameter of d = 0.067 m, inlet width of b = 0.067 m and an inlet radius of r_{ in } = 0.174 m corresponding to an approach flow geometric factor α = 2.688.
Three test cases were analysed coinciding with a flow of Q = 0.725, 1.677 and 3.111 l/s from which tangential and freesurface profile data was available from the experimental test rig to validate the simulation. The flow field was modelled transiently using an implicit second order accurate time differencing scheme at time steps of 0.01 s. The models were initialised using the results from a steady state model and simulation time was up to 40 seconds. The simulations were computed using a the FIONN supercomputer system at the Irish Centre for High End Computing (ICHEC) with 96 to 120 computer cores taking up to 48 hours to compute. Maximum errors in predicting the primary tangential velocity field and freesurface were found to be in the range of 12% and 22% respectively. Additional information on the simulations performed in this study can be found in^{62}.
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Acknowledgements
The authors acknowledge MetFlow SA in Lausanne, Switzerland for having provided the UDP monitor and a number of ultrasonic transducers; the School of Engineering and Architecture of Fribourg, Switzerland for having made available additional ultrasonic transducers; while most of the transducers were provided from the Laboratory of Hydraulic Construction at the EPFL. The project was part funded by the Irish Research Council. The Department of Civil Engineering and Construction, and the Centre for Precision Engineering, Materials & Manufacturing research (PEM) Centre (both IT Sligo) and the Laboratory of Hydraulic Constructions at the EPFL also provided funding for the work. The authors would also like to express gratitude to the Irish Centre for High End Computing for providing simulation time on the FIONN supercomputer during the project. Finally, the authors would also like to thank Dr Eoghan Clifford of the National University of Ireland, Galway for his support while compiling the article and Mr Shane Wimsey for his assistance in performing the laser induced fluorescence experiments.
Author information
Affiliations
Department of Civil Engineering and Construction, Institute of Technology Sligo, Sligo, Ireland
 Sean Mulligan
Laboratory of Hydraulic Constructions (LCH), Ecole Polytechnique Fédérale de Lausanne (EPFL), CH1015, Lausanne, Switzerland
 Giovanni De Cesare
Department of Civil Engineering and Construction, Institute of Technology Sligo, Sligo, Ireland
 John Casserly
Centre for Precision Engineering, Materials and Manufacturing Research and School of Science, Institute of Technology Sligo, Sligo, Ireland
 Richard Sherlock
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Contributions
S.M. contributed by performing initial PLIF measurements on the overall flow field and proposed that it was likely that cellular structures occupied the secondary flow field. He then conceived a link between the behaviour of freesurface vortex and the TaylorCouette flow and proposed that the analogue plays an important role in understanding energy transfer and stability in freesurface vortices. S.M. also engaged heavily in the UDP measurements and numerical simulations and was responsible for experimental design, performing analysis and composing the article. G.C. contributed by recognising the importance of the TaylorCouette flow analogy in its early development and the effect of the circumferential spanning cellular structures on the stability of the vortex flow field. G.C. being one of the early adopters of the UDP instrument conceived an innovative approach to mapping the Taylorvortices using a 7 × 7 array of ultrasound transducers. G.C. was also responsible for analysis of data and editing the article. J.C. contributed by inputting to experimental design, management of the experiments and engaged heavily in the hydraulic analysis. He also contributed to editing the research article. R.S. contributed by recognising the significance of both the mechanical processes in the secondary flow field and its similarities to the classic TaylorCouette flow system. He was responsible for experimental design and overall management of the research team and experiments carried out during the study. He also engaged heavily in data analysis and editing the research article.
Competing Interests
The authors declare that they have no competing interests.
Corresponding author
Correspondence to Sean Mulligan.
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