# Towards a Prototype of a Spherical Tippe Top

Authors: M. C. Ciocci; B. Malengier; B. Langerock; B. Grimonprez
Journal: Journal of Applied Mathematics
 (2012)

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## Abstract

Among spinning objects, the tippe top exhibits one of the most bizarre and counterintuitive behaviours. The commercially available tippe tops basically consist of a section of a sphere with a rod. After spinning on its rounded body, the top flips over and continues spinning on the stem. The commonly used simplified mathematical model for the tippe top is a sphere whose mass distribution is axially but not spherically symmetric, spinning on a flat surface subject to a small friction force that is due to sliding. Three main different dynamical behaviours are distinguished:tipping, nontipping, hanging, that is, the top rises but converges to an intermediate state instead of rising all the way to the vertical state. Subclasses according to the stability of relative equilibria can further be distinguished. Our concern is the degree of confidence in the mathematical model predictions, we applied 3D printing and rapid prototyping to manufacture a “3-in-1 toy” that could catch the three main characteristics defining the three main groups in the classification of spherical tippe tops as mentioned above. We propose three designs. This “toy” is suitable to validate the mathematical model qualitatively and quantitatively.


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## Body

## 1. Introduction

Spinning toys are among the most ancient toys, and there is a great variety of them. It is quite simple to start spinning objects like a top or a gyroscope, and though it is simple to explain their motion in general, it is challenging to write down the detailed equations of motion. Among spinning objects, thetippe top exhibits one of the most bizarre and counterintuitive behaviours. The commercially available tippe tops, patented in Denmark in the 50s, basically consist of a section of a sphere with a rod. After spinning on its rounded body, the top flips over and continues spinning on the stem. It is the friction with the bottom surface and the position of the center of mass below the centre of curvature that cause the tippe top to rise its centre of mass while continuing rotating around its symmetry axis (through the stem). See Figure 1 for an illustration. Remarkably, at the inverted state, the center of mass lies higher than at the initial condition, defying gravity. Experimentally, it is known that such a transition occurs only if the initial spin exceeds a certain critical threshold.Figure 1
The tippe top, showing inversion.The commonly used simplified mathematical model for the tippe top is a sphere whose mass distribution is axially but not spherically symmetric, spinning on a flat surface subject to a small friction force that is due to sliding. Adopting a bifurcation theory point of view we reach a global geometric understanding of the phase diagram of this dynamical system. According to the eccentricity of the sphere and the Jellett invariant (which includes information on the initial angular velocity) six main classes of tops can be identified within three main groups according to the distinguished dynamical behaviours:tipping, nontipping, and hanging; see Figure 3. Note that objects displaying inversion properties such as the tippe top have been known since the 1800s, see, for example, [1]. After the type of tippe top as in Figure 1 was introduced in Denmark, several theoretical articles have been published since then, see, for example, [2–6] for a survey of the literature. Since it was established that sliding friction was necessary to explain the tippe top inversion [2, 7, 8], many studies have been dedicated to the analysis of models for tippe tops, involving linear stability analysis of the relative equilibria, numerical simulations, and so forth. Some studies have addressed the occurrence of transitions between rolling and sliding during the motion, see [3, 4, 9]. In this paper the presented mathematical results mainly reproduce those in [10–15] but our approach is inspired by the hands-on numerical approach as first attempted by Cohen in [2]. We believe this approach is the best choice in giving a clear view of the role of the different parameters that is necessary during the design process of an actual three-dimensional object that effectively demonstrates the model. We remark that in the mathematical model we stick to the common assumption that the only external force acting on the system consists of a normal reaction force and a frictional force of viscous type opposing the motion of the contact point in the supporting plane. This is the most common assumption in the literature, though in [4] the inclusion of a nonlinear Coulomb-type friction is discussed. It is shown there by numerical simulations that the Coulomb term contributes to the tippe top inversion but the effect is weaker compared to the viscous term. The nonlinear Coulomb term results in algebraic destabilization of the initially spinning top, whereas the viscous friction gives exponential destabilization, see also [5]. This argument motivates our choice of including viscous friction only.The phase diagram and bifurcation diagrams illustrate the main results that confirm the findings described in [10]; the type of asymptotic dynamics is a function of the Jellett invariant (which includes information on the initial angular velocity) and eccentricity of the sphere. Either the asymptotic state is unique or the system is bistable. Three main different regimes are distinguished: no tippe top phenomenon occurs no matter what the initial spin is, tippe top dynamics may occur if the Jellett invariant (which is proportional to the initial spin) is sufficiently large, or incomplete tippe top behaviour occurs, where the top rises but converges to an intermediate state instead of rising all the way to the vertical state.We underline that though the classification results can be obtained in a less cumbersome way by using the Routhian reduction as in [10], the approach used in this paper is standard and straightforward to implement from a prototyping point of view. Also, it is amenable for extensions to include for example transitions from sliding to rolling and vice versa. Our concern in this paper is the degree of confidence in the mathematical model predictions. We wanted to be sure that the mathematical model as presented here and in [10] reflected the reality. Our goal was to investigate if it was possible to make a “3-in-1 toy” that could catch the three main characteristics tipping, nontipping,andhanging that define the three main groups in the classification of spherical tippe tops as mentioned above. As far as we know such a toy does not exist yet. We successfully applied the methodology for efficient use of prototyping during the design process as presented in [16]. To the best of our knowledge this is the first time that 3D printing and rapid prototyping is being applied to design and to produce a “toy” suitable to validate the qualitative and quantitative mathematical model describing the behaviour of a dissipative nonlinear dynamical system. From the bifurcation diagram it was clear that it should be possible to hit three out of the 6 classes of tippe tops (one type for each main group) by keeping one of the characterizing parameters of the system fixed and varying the other. We believe that the realization of an actual toy is a more powerful validation of the model than software simulations which are directly affected by the underlying mathematical idealization assumptions.Since the two parameters on which the whole classification is based,inertia ratio and eccentricity, are not independent, the challenge was to come up with a feasible prototype which could be easily mechanically driven. After detailed mathematical calculations and the development of 3D animations (see electronic attachments or http://cage.ugent.be/~bm/tippetop/tippetop.html) we used 3D printing to create a functional model giving us a quick and easy hands-on demonstration capability.


## 2. Mathematical Results

In this paper we consider a sphere whose mass distribution is axially but not spherically symmetric, spinning on a flat surface subject to a small friction force that is due to sliding. In [13], Ebenfeld and Scheck presented a detailed analysis of the dynamics of the eccentric spinning sphere on a flat surface where friction is assumed to be only due to sliding, see also [14]. Without making any other assumptions, we show that their results imply a full qualitative understanding of the asymptotic long-term dynamics. Whereas the treatment of [13, 14] is mainly analytical, here we adopt a bifurcation theory point of view leading to a global geometric understanding of the phase diagram. The phase diagram in Figure 2 and bifurcation diagrams in Figure 3 illustrate our main results. Recall that an ω-limit set of a dynamical system is a closed invariant set that is accumulated by a (forward) trajectory [17]. Our main result is summarized in the following theorem.Figure 2
Phase diagram for the dynamics of the eccentric sphere with small sliding friction. The regions of the phase diagram correspond to the qualitative types of bifurcation diagrams ofSO(2)×SO(2) relative equilibria in Figure 3.Figure 3
Qualitative bifurcation diagrams ofSO(2)×SO(2) relative equilibria, for the different regions in the phase diagram of Figure 2. Solid black branches correspond to stable relative equilibria, while dashed black branches correspond to unstable ones. The vertical states θ=0 and θ=π always exist, from which intermediate states (with 0<θ<π) may branch off.Theorem 2.1.
A spinning eccentric sphere on a flat surface with small slipping friction admits three types of (asymptotically stable)ω-limit sets:(i)
vertically spinning top (θ=0), which has its center of mass straight below its geometric center,(ii)
vertically spinning top (θ=π), which has its center of mass straight above its geometric center,(iii)
intermediate spinning top (0<θ<π), whose center of mass is neither straight below nor straight above its geometric center.These are solutions of constant energy that are purely rolling  due to the assumption on sliding friction (i.e., they display no slipping). The vertical states are periodic, whereas, in general, the intermediate states are quasiperiodic.
At most two of the above types of solutions can be stable at the same time. In case the stable solution is unique its basin of attraction consists of almost the entire phase space (subset of full measure). If the system is bistable, the separatrix between the two different domains of attraction for the asymptotically stable states is expected to be formed by the stable manifold of an unstable intermediate spinning top solution.All the analytical results needed to arrive at this conclusion can in principle be found in [13, 14]. However, these papers stop short of drawing the full global conclusions as formulated in the above theorem, and also crucially they did not present the phase diagram and bifurcation diagrams that we present in Figures 2 and 3.We note that for the eccentric sphere in regime I, the stateθ=0 is always asymptotically stable and thus does not display the tippe top phenomenon. Similarly, no such dynamics arises in regime III since there the inverted state θ=π is always unstable. Tippe top dynamics may occur in regime II if the Jellett invariant (which is proportional to the initial spin) is sufficiently large, corresponding to the empirical observation that tippe top dynamics requires a sufficiently large initial spin. In the subregimes IIb and III it is also possible to observe incomplete tippe top behaviour, where the top rises but converges to an intermediate state instead of rising all the way to the vertical state θ=π. Note that, in regime I, tipping might occur if the top is initially spun sufficiently fast under an angle not close to θ=0.It is important to recognize the existence of symmetries. Recall that symmetries are transformations of the phase space that map solutions of a system to other solutions. In our model of the eccentric sphere on a flat surface, symmetries arise due to the homogeneity of the surface on which the sphere moves and the rotational symmetry of the eccentric sphere. The combined symmetries are thus the Euclidean groupE(2) (acting as translations and rotations in the xy plane) and the rotation group SO(2) acting as rotation of the sphere around its axis of symmetry.It turns out that theω-limit sets mentioned above are all relative equilibria with respect to the symmetry group SO(2)×SO(2)<E(2)×SO(2), see Section 4. Recall that relative equilibria with respect to a group Σ are equilibria for the associated flow on a reduced phase space that is obtained from the original phase space by taking the quotient with respect to the action of Σ. The existence and type of such relative equilibria depend solely on the inertia ratio, the eccentricity of the sphere, and the Jellett integral of motion. We identify a number of regimes characterizing the relative equilibria as a function of the Jellett invariant (which is proportional to the initial angular velocity). The vertical states θ=0 and θ=π are always SO(2)×SO(2) relative equilibria and their stability depends on the inertia ratio, the eccentricity of the sphere, and the Jellett integral of motion. In addition, intermediate states may exist, which branch off from the vertically spinning solutions. We sketch the phase diagram in Figure 2. For the labeled regions in this phase diagram, the corresponding bifurcation diagrams for the relative equilibria are presented in Figure 3.The proof of Theorem2.1, which builds upon the results by [13, 14], can be found in the appendix. In order to present our point of view clearly and in a self-contained way, in Section 3 we also present a derivation of the equations of motion of the eccentric sphere model of the tippe top, including a discussion of the symmetries and their consequences. Here also, one finds a precise description of the assumed nature of the friction and a definition of all the relevant variables that appear as parameters in Figures 2 and 3. In Sections 4 and 5 the relative equilibria of the system and their stability are discussed. The readers who are acquainted with the topic can start reading from Section 6.We would like to point out that the strategy of proof used here may well be applicable to a large number of similar examples of mechanical systems under the influence of some kind of friction, such as theRattleback [18] or Hycaro tippe top of Tokieda [19]. The key observation is that for mechanical systems under the influence of friction, in a natural way the energy becomes a Lyapunov function since friction causes energy loss. The next observation is that orbits which do not dissipate energy need to lie entirely on a subvariety of the phase space that is defined by the condition that friction is absent. Equilibria naturally lie on this subset since they have zero velocity and friction is absent at zero velocity. However, one would expect that typically no solution lies entirely on this subvariety, unless the solution lies on the orbit of a symmetry group that leaves the zero friction subvariety invariant. (One can make this precise by constructing a small local perturbation that moves a solution off the zero friction subvariety.) In many cases, the set of such relative equilibria can be accurately analyzed, either analytically or numerically, and the local stability properties can be deduced from a dissipation-induced instability point of view, based on the local stability properties of the relative equilibria in the absence of friction. We note in this respect that the set of ω-limit sets on the zero friction subvariety is independent of the form and size of the friction. The final step is to draw global conclusions from this local information. The latter is within reach if one has a good understanding of the ω-limit sets. We would like to stress that Theorem 2.1 concerns the asymptotic dynamics. In an experiment with small friction, the observation may well be dominated by transient dynamics which bears strong resemblance (on short time scales) to the dynamics of the spherical top without friction. The dynamics of the latter is rather complicated as it is a nonintegrable Hamiltonian system. In Section 7 we present some results from numerical simulations demonstrating explicitly some examples where the transient dynamics does not appear to prevent fast convergence to the asymptotic states (although of course for sufficiently small friction coefficient the transient dynamics would dominate on finite time intervals).


## 3. The Equations of Motion

We consider aneccentric sphere as in Figure 4, where O denotes the center of mass and 𝒞 the center of the sphere. The line joining the center of mass and the geometrical center is an axis of inertial symmetry: in the plane perpendicular to this axis the moment of inertia tensor of the sphere has two equal principal moments of inertia.Figure 4
Eccentric sphere version of the tippe top.R is the radius of the sphere, the center of mass O is off center by ϵ. The top spins on a horizontal table with point of contact Q. The axis of symmetry is Oz and the vertical axis is OZ, they define a plane Π (containing OQ) which processes about OZ with angular velocity φ̇. The height of O above the table is h(θ).We describe the motion of the sphere using three reference frames:(I)
an inertial (laboratory) frameMxyz, where M is some point on the table and the z-axis is the vertical.(II)
a (noninertial) rotating frameOXYZ whose origin is in the center of mass O and whose 3rd axis is always parallel to the vertical. The X and Y axes are specified below.(III)
a principal axis systemOxyz, whose z-axis is the symmetry axis of the sphere (Note that in [5] the origin of the reference frames (II) and (III) is at the center of the sphere, and not at the center of mass.)The reference frames (II) and (III) are indicated in Figure4. The eccentricity ϵ is the distance between the center of mass O and the geometric center 𝒞 of the sphere, with 0<ϵ<R, where R denotes the radius of the sphere. We denote the moments of inertia Ix=Iy=:A and Iz=:C. The point of contact with the plane of support is denoted by Q.Let(θ,φ,ψ) be the Euler angles of the body with respect to OZ, see Figure 5 for an illustration. The OzZ-plane Π contains the vector q=OQ which joins the center of mass to the point of contact. The plane Π is inclined at angle φ to the vertical Mxz-plane and processes with angular velocity φ̇ around the vertical OZ. We choose the horizontal OX in Π so that OY is perpendicular to Π. For the rotating frame, Ox is in Π and perpendicular to the symmetry axis Oz and the axis Oy coincides with OY. (Note that the axes Ox and Oy are principle axes, but they are not body fixed.) The angle between the vertical OZ and the axis Oz of the top is denoted by θ. The angular velocity θ̇ describes the nutation of the body in the vertical plane Π. The angle ψ describes the orientation of the body with respect to the OXYZ frame and ψ̇ is the spin of the sphere around its symmetry axis. We denote by e1,e2,e3 the unit vectors along OX,OY,andOZ and by i,j,andk those along Ox,Oy, and Oz. Note that e2=j. Because of the inherent translational symmetry (of the body on the plane), it is convenient to describe the body in terms of the relative (moving) reference frames (II) and (III), rather than in the absolute reference frame (I). By doing so we thus ignore the translational motion on the plane and focus on the relative motion of the body, which captures the tippe top behaviour.Figure 5
Euler angles(φ,θ,ψ) to fully determine the body, given the coordinates of the center of mass O in an inertial frame with center M.The (relative) position vector of the body is(3.1)x=xi+yj+zk=Xe1+Ye2+Ze3,
or x=(x,y,z)Oxyz=(X,Y,Z)OXYZ. Note that the coordinates of the reference frames (II) and (III) are related by the relations(3.2)x=Xcos⁡(θ)-Zsin⁡(θ),y=Y,z=Xsin⁡(θ)+Zcos⁡(θ).
The reference frames (II) and (III) rotate with respective angular velocities(3.3)ΩII=(0,0,φ̇)OXYZ=(-φ̇sin⁡(θ),0,φ̇cos⁡(θ))Oxyz,ΩIII=(-φ̇sin⁡(θ),θ̇,φ̇cos⁡(θ))Oxyz.
The angular velocity of the body ω involves, in addition, the angular velocity ψ̇:(3.4)ω=-φ̇sin⁡(θ)i+θ̇j+nk=ψ̇sin⁡(θ)e1+θ̇e2+(φ̇+ψ̇cos⁡(θ))e3=(n-φ̇cos⁡(θ))sin⁡(θ)e1+θ̇e2+(φ̇sin⁡2(θ)+ncos⁡(θ))e3,
where n:=ψ̇+φ̇cos(θ) denotes the component of ω about Oz, better known as the spin. For later use we introduce the notation ω=(ωi,ωj,ωk). Consequently, with I denoting the inertia tensor of the sphere, the angular momentum of the sphere is given by(3.5)L=Iω=-Aφ̇sin⁡(θ)i+Aθ̇j+Cnk=(Cn-Aφ̇cos⁡(θ))sin⁡(θ)e1+Aθ̇e2+(Aφ̇sin⁡2(θ)+Cncos⁡(θ))e3.
The point of contact Q has coordinates(3.6)Q=(-h2(θ)ddθ(cos⁡(θ)h(θ)),0,-h2(θ)ddθ(sin⁡(θ)h(θ)))Oxyz=(ϵsin⁡θ,0,ϵcos⁡θ-R)OXYZ=(Rsin⁡θ,0,ϵ-Rcos⁡θ)Oxyz.
The velocity of the point of contact Q is(3.7)VQ=vO+ω×q,
where q=OQ denotes the vector from the center of mass O to the point of contact Q and vO is the velocity of the center of mass. We set vO=Ue1+Ve2+We3 and use the fact that Q=(h′(θ),0,-h(θ))OXYZ to obtain(3.8)ω×q=(-θ̇h(θ),sin⁡(θ)(ϵφ̇+Rψ̇),-θ̇h′(θ))OXYZ=(-θ̇h(θ),sin⁡(θ)(ϵφ̇+R(n-φ̇cos⁡(θ))),-θ̇h′(θ))OXYZ.
Hence, we obtain(3.9)VQ=(U-θ̇h(θ),V+sin⁡(θ)(ϵφ̇+R(n-φ̇cos⁡(θ))),W-θ̇h′(θ))OXYZ.
The fact that the sphere remains in contact with the table is expressed by the (holonomic) constraint(3.10)zO=h(θ)=R-ϵcos⁡(θ),
where h(θ) denotes the height of the center of mass O above the table, compare Figure 4. From this constraint it follows that the e3 component of v0 is(3.11)W:=ddtz0=θ̇h′(θ)=ϵθ̇sin⁡(θ)
so that the Z-component of VQ vanishes, consistent with the constraint.We note that the physical interpretation ofVQ concerns the phenomenon of slipping. In case VQ≠0 the body slips on the surface. In contrast, a rolling motion of the body is characterized by the fact that VQ=0.The equations of motion will be derived, in Newton’s spirit, as a consequence of the action of external forces. We distinguish the following forces acting on the sphere(i)
The gravitational force:G=-mge3, where m is the total mass of the sphere.(ii)
A forceFQ=Rn+Rf acting on the point of contact Q, where Rn=Rne3, is the normal reaction force at Q (due to the stiffness of the surface) and Rf is a friction force. For completeness we mention [20] where a mathematical model for the tippe top is proposed taking elasticity properties of the table and tippe top into account.Friction is the resistive force acting between bodies that tends to oppose and damp out motion. Friction is usually distinguished as being either static friction (the frictional force opposing placing a body at rest into motion) or kinetic friction (the frictional force tending to slow a body in motion). Importantly, we assume that the friction force is entirely due to the slipping of the sphere on the surface and neglect all other sources of friction. Friction forces can be complicated, and there are various models in circulation. We adopt the assumption ofviscous friction [9, 15, 21] and assume the friction force to be given by(3.12)Rf=-μRnVQ,
where μ is the coefficient of sliding friction with the dimension of (velocity)−1. Rf is proportional to the size of the normal reaction force and vanishes smoothly when VQ→0. (An alternative model for the friction force is the so-called Coulomb friction Rf=-μRn(VQ/|VQ|). This model is not appropriate when VQ→0 due to the singular nature of this force when VQ=0.) Euler’s equations of motion for the sphere,(3.13)dLdt+Ω×L=q×FQ,
govern the evolution of the angular momentum L in a noninertial reference frame, rotating with frequency Ω, due to the influence of the external torque q×FQ. The equation of motion for the center of mass O in the rotating frame is(3.14)m(dvOdt+Ω×vO)=-G+FQ.
In terms of the coordinates in reference frame (III) the equations of motion (3.13) yield(3.15)Aφ̈sin⁡(θ)=(Cn-2Aφ̇cos⁡(θ))θ̇+zQFY,Aθ̈=-φ̇sin⁡(θ)(Cn-Aφ̇cos⁡(θ))+ZQFX-XQRn,Cṅ=xQFY,
where Q=(xQ,yQ,zQ)Oxyz=(XQ,YQ,ZQ)OXYZ and FQ=(FX,FY,FZ)OXYZ. From the equation for the motion of the center of mass (3.14), in terms of reference frame (II), we obtain(3.16)m(U̇-φ̇V)=FX,m(V̇+φ̇U)=FY,mẆ=Rn-mg.
Recalling that W=θ̇h′(θ), from the last of the latter equations we may derive an expression for Rn:(3.17)Rn=mg+mddt(θ̇h′(θ))=mg+mϵ(θ̈sin⁡(θ)+θ̇2cos⁡(θ)).
The equations of motion (3.15) and (3.16) can be written as a system of six coupled first-order nonlinear ordinary differential equations in the variables (u,v,α,φ,β,θ,n), where α:=φ̇, β:=θ̇, u:=mU, and v:=mV.Settingm=1 for simplicity, these may be arranged in the standard form ḃ=f(b) (when sin(θ)≠0)(3.18)α̇=1sin⁡(θ)[CAnβ-2αcos⁡(θ)β+zQFYA],β̇=1A[αsin⁡(θ)(Aαcos⁡(θ)-Cn)-RnXQ+ZQFX],θ̇=β,ṅ=xQFYC,u̇=αv+FX,v̇=-αu+FY,φ̇=α,ψ̇=n-αcos⁡(θ).
It should be remembered that Rn, FX, and FY are still functions of the other variables. For instance, from (3.17) and (3.18) one finds(3.19)Rn=g+β2h′′(θ)+h′(θ)αsin⁡(θ)(αcos⁡(θ)-Cn/A)1+h′(θ)/A[-h(θ)μ(U-βh(θ))+h′(θ)].
Recall that we require that Rn≥0. If this condition fails, the sphere loses contact with the surface. Expressions for FX and FY follow similarly from (3.12).It is important to recognize that some of the structure of the equations of motion (3.18) is due to symmetry. We recall that the symmetries are the Euclidean group E(2) (acting as translations, rotations, and reflections in the Mxy plane) and the rotation group SO(2) acting as rotation of the sphere around its axis of symmetry. The effect of the Euclidean symmetry is that the right-hand side of the equations of motion contain no reference to the position of the sphere on the surface. In a similar way, due to the rotational symmetry the equations of motion do not depend explicitly on φ. The system can be viewed as three coupled systems, where the coupling is of skew product type: the evolution of α,β,θ, and n does not depend on u,v, and φ, and the evolution of u, and v does not depend on φ. Moreover, note that the position of the center of mass relative to the surface (in Mxy coordinates) could in principle be obtained by integrating the velocities u and v over time. Because of the fact that we take friction into account, Noether’s theorem does not apply, so the continuous symmetries we observe need not (and do not) give rise to conserved quantities. However, it was discovered by Jellett [8] by an approximate argument, and later proved by Routh [6], that the system (3.18) has the following conserved quantity:(3.20)J=-L⋅q.
Indeed, it follows from (3.13) that (dL/dt+Ω×L)⊥q, so that(3.21)ddtJ=-L⋅(ddtq+Ω×q)=-(Cn-Aφ̇cos⁡(θ))h′(θ)2ddt(sin⁡(θ)h′(θ))︸=0=0.
Note that the Jellett invariant can be written as ([10, 15, 21])(3.22)J=Cn(Rcos⁡(θ)-ϵ)+Aφ̇Rsin⁡2(θ).


## 4.ω-Limit Sets Are Relative Equilibria

Our aim is to describe the asymptotic dynamics of the eccentric sphere. Recall that a subset of the phase space is anω-limit set if this set is accumulated by (forward) orbits. While the friction force destroys the Hamiltonian nature of the dynamics, it greatly simplifies the asymptotic dynamics. This follows from the fact that in the presence of friction the energy, which is conserved in the absence of friction, is almost always decreasing along solutions.The energy is given byE=T+V, where T=Trot+Ttr is the kinetic energy with its rotational and translational part and V=mgh(θ) is the potential energy. With our choice of variables we may write Trot=(1/2)(Aωi2+Aωj2+Cωk2) and Ttr=(1/2)m(ẋ2+ẏ2+ż2), where ż=ϵmsinθθ̇.Lemma 4.1 (see [13]).
The energyE is a Lyapunov function (recall that a Lyapunov function is nonincreasing along orbits) for (3.18). In particular,
(4.1)ddtE=VQ⋅Rf≤0.AsRf is parallel (and opposite) to VQ, (d/dt)E vanishes if and only if VQ vanishes. Observe that E(t) decreases monotonically and hence is a suitable Lyapunov function. Moreover, E(t) is analytic and therefore along orbits it is either strictly decreasing or constant. The energy E is constant only if VQ=0, that is in the absence of friction. Thus, the ω-limit sets must consist of orbits which do not experience friction. We show that such orbits are necessarily relative equilibria.Proposition 4.2.
Solutions have constant energy only if they are relative equilibria with respect to the action ofSO(2)×SO(2).Proof.
We already concluded thatVQ needs to be equal to 0 along any orbit in an ω-limit set. A straightforward calculation shows that VQ=(d/dt)VQ=0 indeed implies that ϕ̇=Ẋ=0, so that such a solution must be an SO(2)×SO(2) relative equilibrium.This observation is in fact what one would generically expect to find. IfM is a submanifold of the phase space that corresponds to the absence of friction, in general it would be quite unexpected to find a nonequilibrium solution that lies entirely inside M.


## 5. Stability and Bifurcations of Relative Equilibria

Having determined that the relative equilibria are the only possible asymptotic states in the presence of friction, we derive in this section these solutions of constant energy using the explicit equations of motion (3.15)-(3.16), see also [5, 13, 15]. With φ̇=constant and VQ=0,Rf=0, the equations of motion yield α̇=0, β̇=0, β=0, ṅ=0, U=0, W=0 and(5.1)αV=0,αsin⁡(θ)(Aαcos⁡(θ)-Cn)-mgϵsin⁡(θ)=0,V+[R(n-αcos⁡(θ))+ϵα]sin⁡(θ)=0.
These equations have the following three types of solutions. The linear stability analysis differs from [13, 14] in methodology.Vertical States
(1)
Vertical stateθ=0:
(5.2)U=V=0,θ=0,n=arbitraryconstant,α=φ̇=undefinedconstant.
The top is spinning about its axle with center of mass straight below the geometric center.(2)
Vertical stateθ=π:(5.3)U=V=0,θ=0,n=arbitraryconstant,α=φ̇=arbitraryconstant.
The top is spinning about its axle with center of mass straight above the geometric center.Intermediate States
For these solutions we haveU=V=0, 0<θ<π, and n,α,andθ are related by
(5.4)n=αcos⁡(θ)-ϵRα,(5.5)α(Aαcos⁡(θ)-Cn)-mgϵ=0.
Elimination of n from the above yields
(5.6)α2=mgϵ(A-C)cos⁡(θ)+C(ϵ/R).
Hence, the condition for the existence of intermediate states is
(5.7)(AC-1)cos⁡(θ)+ϵR>0.It is natural to divide the solutions into three groups, according to regimes of the parametersA/C and ϵ/R [21].Group I:A/C<1-ϵ/R. Intermediate states exist with
(5.8)θ>θc1=cos⁡-1(ϵ/R1-A/C),with0<θc1<π2.Group II:1-ϵ/R<A/C<1+ϵ/R. Intermediate states exist with any 0<θ<π.Group III:A/C>1+ϵ/R. Intermediate states exist with
(5.9)θ<θc2=cos⁡-1(ϵ/R1-A/C),withπ2<θc2<π.As in [10] we further refine this classification. Note that the intermediate states discussed here correspond to the tumbling solutions discussed in [13].The intermediate states are completely determined by (5.4), (5.5), and the Jellett invariant J. More precisely, combining the square of (3.22) with (5.4) and (5.6), they are obtained by solving(5.10)f(J2,cos⁡θ):=J2mgϵCR2[(AC-1)cos⁡(θ)+ϵR]-[(cos⁡(θ)-ϵR)2+AC(1-cos⁡2(θ))]2=0.
The next theorem summarizes the linear stability and local bifurcation results, as depicted in Figure 3 (cf. [21]), and the proof is sketched in the Appendix. We identify six different groups according to how the value of A/C is related to the eccentricity ϵ/R. In the literature, results have previously been expressed in terms of variables n0 and nπ, referring to the spin of an initial condition in a vertical state. We define n0:=J/C(R-ϵ), which is the value of the spin n at θ=0 for motion with Jellett invariant J. Similarly, nπ:=-J/C(R+ϵ) denotes the spin of the solution with Jellett invariant J at θ=π. Note that, for a fixed value of the Jellett invariant J, these spins are related by n0=-nπ(R+ϵ)/(R-ϵ). We further define(5.11)n±:=±mgϵC[(1±ϵ/R)-A/C](1±ϵ/R),b:=ϵ/R-(1/3)A/C(1-A/C-(ϵ/R)2)1-A/C,
and θb:=arccos(b). Furthermore we define c=ϵ/R/1-(A/C) and θc:=arccos(c).Theorem 5.1.
The bifurcation diagrams of the eccentric sphere spinning on a flat surface with small friction fall in one of the following six categories (Figure3).Group I:A/C-1<-ϵ/R.
(i)
The vertical stateθ=0 is stable for any value of J.(ii)
The vertical stateθ=π is stable if |nπ|>n+ and unstable otherwise.(iii)
Intermediate states exist for all values ofθ satisfying θ>θc.Group Ia:b<-1. The entire branch of intermediate states is unstable.Group Ib:b>-1. The branch of intermediate states has a fold point at θ=θb. The branch with θ>θb is stable, while the branch with θ<θb is unstable.
Group II:-ϵ/R<(A/C-1)<ϵ/R.
(i)
The vertical stateθ=0 is stable if |n0|<n- and unstable otherwise.(ii)
The vertical stateθ=π is stable if |nπ|>n+ and unstable otherwise.(iii)
Intermediate states exist for allθ. We distinguish the following three subgroups.Group IIa:(A/C-1)<-(ϵ/R)2  and |b|<1. A fold bifurcation of intermediate states occurs.Group IIb:(A/C-1)>-(ϵ/R)2  or b>1. The entire branch of intermediate states is stable.Group IIc:(A/C-1)<-(ϵ/R)2  and b<-1. The entire branch of intermediate states is unstable.
Group III:(A/C-1)>ϵ/R.
(i)
The vertical stateθ=0 is stable if |n0|<n-.(ii)
The vertical stateθ=π is unstable for all J.(iii)
Intermediate states exist forθ<θc and are all stable.The proof of Theorem5.1 can be mainly recovered from [10]; for completeness we provide the calculations based on a direct approach in the appendix.


## 6. Prototype of a Spherical Tippe Top

Rapid prototyping (RP) technologies enable solid models to be obtained from designs generated with CAD applications. Their increasing popularity in industry is due to the reduction in cost and time associated with the use of these models when verifying product development stages and improvements in end quality. These technologies can also be applied to verify the correctness and/or accuracy of mathematical models and last but not least to enhance students’ active learning in the frame of a learning-by-doing approach. Students can bring their designs to fruition and develop a deeper insight in abstract concepts. We made a prototype of a spherical tippe top for educational use in the Product Development Laboratory of Howest.As pointed out earlier, to realize a 3-in-1 toy an axially symmetric sphere where one has control overA/C and ϵ/R is needed. We considered three possible designs:(1)
a solid sphere with a cylindrical hole through the center where a setscrew can move;(2)
a hollow sphere with a cylindrical rod on which a weight can move;(3)
a hollow sphere with a toroidal band at the equator fitted with a cylindrical rod on which a weight can be screwed.From the bifurcation diagram in Figure2, it is clear that it is possible to hit the three main groups by fixing ϵ/R and changing A/C. Therefore, it is important to understand for the three designs how A/C and ϵ vary with respect to each other when the weight is moved. We set up a Maple worksheet based on the given mathematical description and calculated A/C and ϵ in function of the position of the midpoint of the moving weight with respect to the center of the sphere; this will be further on denoted by Z2. We took into account the physical parameters: dimensions of the different parts (radii, heights, and thickness) and the density of the materials.From this we realized that for the solid sphere the goal of the three types is within reach, whereas for the hollow sphere the design has to be modified. Our modifications resulted in the third design as given above. We now discuss our findings for the realized prototypes. Our realizations were all printed with the commercial available Dimension SST1200es with printing technology based on the FDM principle (fused deposition modeling) in ABSplus.


### 6.1. Sphere with Cylindrical Hole and Setscrew

For the first design we realized three different tops, varying the geometrical dimensions. This was done because the calculation showed that for the given materials some zones are hard to achieve or are very narrow, see Figure7. The prototype consists of a sphere with a cylindrical hole through the center, together with a piece of adjustable cylindrical iron wire (setscrew), see Figure 6. With a caliper, it can be checked how deep the setscrew is set in the hole. The position of the midpoint of the setscrew with respect to the center of the sphere is denoted by Z2. The hole is suitable for a setscrew M12. The dimensions of the toy were chosen based on the mathematical calculations derived from the model. The diameter of the sphere was chosen so that one can comfortably spin the toy by hand. With a sphere of diameter 50 mm, good values for the chosen design are a hole of radius 5.5 mm, filled with the setscrew of height 15 mm, or a hole of radius 1.5 mm, filled with the setscrew of height 3 mm, see Figure 7. The densities are 1.08 g/cm3 for ABSplus and 7.87 g/cm3 for the setscrew.First prototype of a spherical tippe top.
(a)(b)Different tippe top regimes in function of the positionZ2 of the midpoint of the setscrew. The black lines are ±ϵ(Z2)/R, the blue curve is A(Z2)/C-1, and the red curve is -(ϵ(Z2)/R)2. On the left, the result for the printed prototype with a M12 setscrew, see Figure 6. On the right, the result for a prototype of the same shape but a setscrew M3.
(a)(b)The prototype is axially symmetric; therefore, only the eccentricityϵ and the moment of inertia A are functions of Z2, they are easily calculated; C remains constant when moving the setscrew up and down. In Figure 7 the quantities (A/C)-1, ±ϵ/R, and -(ϵ(Z2)/R)2 are plotted as functions of Z2, (a) for the prototype with a M12 setscrew and (b) for the prototype with a M3 setscrew. The printed prototype in Figure 6, is of the first type and according to the mathematical calculations will exhibit the predicted behaviour as follows: for Z2 between 0mm and 7.95mm the toy does not show tippe top dynamic no matter what the initial spin is (type I), for Z2 between 7.95mm and 17.76mm complete tippe top dynamic is observed (type IIc). For Z2 above 17.76mm the top is of type IIb (incomplete tipping is observed if initial spin is not sufficiently high).For the different positions of the weight, we launched by hand the toy plenty (≥50) of times and registered each time tipping, nontipping, or hanging. In Table1 we report the typical results for 5 launches. Note that the tippe top is hand spun, so there will be a deviation from the starting position θ=0. Tipping and nontipping were mostly observed in the setup of type IIa and I, respectively. For the setup of type IIb, the expected behaviour (tipping) was not observed; we always observed the hanging behaviour. This is because we were not able to launch the toy fast enough by hand and also because the setscrew sticking out the toy does not allow ideal launching position. Our observations indicate that the prototype behaves as predicted by the model. In details, tipping and hanging at Z2=5 can be explained by the presence of a branch of intermediate states and stable π position that one could hit if the toy is not launched exactly from the θ=0 position, see Figure 3. The hanging at Z2=15 is due to the fact that we did not launch the top fast enough.Table 1
Hand launched tippe top. Observed occurrences of the different types on 5 launches.
Depth setscrew17.512.57.52.5−2.5Z205101520Nontipping53000Tipping01540Hanging01015TheoryI (sphere)IIIaIIaIIbFor a prototype fit for a M3 screw, the intervals forZ2 are as follows: for Z2 between 0mm and 3.33mm the toy does not show tippe top dynamic no matter what the initial spin is (type I); for Z2 between 3.33mm and 18.20mm complete tippe top dynamic is observed (type II). For Z2 above 18.20mm the top is of type III (incomplete tipping is observed). Also, this prototype was spun ≥50 times, and we registered similar observations as for the previous one.We conclude that this prototype can give a working 3-into-1 toy but has some disadvantages.(i)
The setscrew can come loose after intensive use.(ii)
When there are three zones present, at least one of the zones is small.(iii)
Using a caliper to know if the setscrew is in the center is not practical.Several attempts were done in the computations to improve the design, for example, by adding holes into the solid sphere. These attempts were not successful, so no other prototype was printed. Instead, we concentrated on the sphere with a cylindrical rod.


### 6.2. Sphere with Cylindrical Rod

The second design consists of a spherical shell with a cylindrical solid rod through the center along which a symmetric bead is spun; this bead can be put at different heights along the rod. In this design, the user must open the sphere and change the position of the weight by screwing it up or down, after which the sphere can be closed and spun. See Figure8.Figure 8
Design of the second prototype.The advantage of this design is that different ABS colors can easily be used for both sides making the tipping more visible and that the rod can be marked at the critical positions. Where in the first design setscrews of different length can be used, in this design weights of different lengths and different widths can be considered within one toy. Also, different materials for the rod can be considered.However, computations show that a 3-into-1 toy was difficult to obtain with the chosen materials: ABS, iron, and nylon. We briefly summarize our findings that form the basis of further improvements that lead to the third prototype. We tried three different possibilities for the rod: iron, nylon, and ABS. Nylon and ABS seem to work best. With an iron rod and physical parameters that allow easy playing with the toy we did not succeed in catching all the three zones. See below for the specific values of the parameters. As Figure9(a) shows, only zone three is hit, which means that this tippe top never shows complete inversion but may tip up to a certain angle.(a) Different tippe top regimes in function of the position of the midpoint of the setscrew. The black lines are±ϵ(Z2)/R, the blue curve is A(Z2)/C-1, and the red curve is -(ϵ(Z2)/R)2. The physical parameters for the construction are radius of the spherical shell in ABS of 25mm, thickness of the shell of 2.5mm, radius of the iron cylindrical rod of 3mm, radius of the (iron) weight of 10 mm, and height of the weight of 10mm. (b) Different tippe top regimes in function of the position of the midpoint of the setscrew. The black lines are ±ϵ(Z2)/R, the blue curve is A(Z2)/C-1, and the red curve is -(ϵ(Z2)/R)2. The physical parameters for the construction are radius of the ABS spherical shell of 25mm, thickness of the shell of 2.5mm, radius of the nylon cylindrical rod of 2.5mm, radius of the (iron) weight of 10mm, and height of the weight of 10mm.
(a)(b)The prototype is axially symmetric; therefore, only the eccentricityϵ and the moment of inertia A are functions of Z2, they are easily calculated; C remains constant when moving the weight up and down. The physical parameters for the construction are radius of the spherical shell of 25 mm, thickness of the shell of 2.5mm, radius of the cylindrical rod of 3mm, radius of the weight of 10 mm, and height of the weight of 10mm.In the case of a nylon or ABS rod, it was possible to obtain a tipping top. As illustrated in Figure9(b), both zones II and III are hit, which means that complete tipping and incomplete tipping may be observed according to the position of the weight. Note that the section of the blue curve in zone III is very small, which makes it very difficult to observe the hanging phenomenon. A similar observation holds for the section of the blue curve in zone I; this is so small that nontipping behaviour cannot in practice be observed. Many launches of this prototype only confirmed the observations above. This seems to be a good type II tippe top, but we were not able to observe the other behaviours.


### 6.3. Sphere with a Toroidal Band and a Cylindrical Rod

The third design consists of a spherical shell with a toroidal band around the equator and a cylindrical solid rod through the center along which a symmetric bead is spun. Also in this design, the user must open the sphere and change the position of the weight by screwing it up or down, after which the sphere can be closed and spun. See Figure10.Figure 10
Design of the third prototype.Adding a toroidal band was a way to find a compromise between a spherical shell and a solid sphere. The prototype is still axially symmetric, and the band provides a better click system to open and close the toy. The physical parameters for the construction are radius of the spherical shell of25mm, thickness of the shell of 3mm, radius of the cylindrical rod of 3mm, radius of the weight of 6mm, and height of the weight of 10mm. The band has the form of a solid of revolution generated by an ellipse rotating around the rod, the semiaxes of the ellipse measure, respectively, 7mm and 4mm. The rod is made of iron. According to the mathematical model, the top should behave as follows: for Z2 between 0mm and 4.14mm the toy does not show tippe top dynamic (type I); for Z2 between 4.14mm and 16.8mm complete tippe top dynamic is observed (type II). For Z2 above 16.8mm the top is of type III (incomplete tipping is observed).The toy was launched many times, allowing to observe without problems zones I and II predicted by the model. Zone III is, however, difficult to observe at first, the maximumZ2 that can be obtained with the constructed prototype was only 15 mm (due to the fastening system of the rod), and moreover θc>2π/3 which is not so easy to see. Different weights can, however, be used so that zone III becomes visible; for example, this is the case when using an iron weight with radius 8mm and height 5mm. We conclude that this last prototype is a good candidate for the 3-in-1 toy, although some further optimizations of the physical parameters can be considered (Figure 11).Figure 11
Different tippe top regimes in function of the position of the midpoint of the setscrew. The black lines are±ϵ(Z2)/R, and the blue curve is A(Z2)/C-1, the red curve is -(ϵ(Z2)/R)2. The physical parameters for the construction are here: radius of the ABS spherical shell 25mm, thickness of the shell 3mm, radius of the cylindrical rod 3mm, radius of the (iron) weight 6mm, height of the weight 10mm, semi-axis of the ellipse generating the torus 7mm and 4mm.


## 6.1. Sphere with Cylindrical Hole and Setscrew

For the first design we realized three different tops, varying the geometrical dimensions. This was done because the calculation showed that for the given materials some zones are hard to achieve or are very narrow, see Figure7. The prototype consists of a sphere with a cylindrical hole through the center, together with a piece of adjustable cylindrical iron wire (setscrew), see Figure 6. With a caliper, it can be checked how deep the setscrew is set in the hole. The position of the midpoint of the setscrew with respect to the center of the sphere is denoted by Z2. The hole is suitable for a setscrew M12. The dimensions of the toy were chosen based on the mathematical calculations derived from the model. The diameter of the sphere was chosen so that one can comfortably spin the toy by hand. With a sphere of diameter 50 mm, good values for the chosen design are a hole of radius 5.5 mm, filled with the setscrew of height 15 mm, or a hole of radius 1.5 mm, filled with the setscrew of height 3 mm, see Figure 7. The densities are 1.08 g/cm3 for ABSplus and 7.87 g/cm3 for the setscrew.First prototype of a spherical tippe top.
(a)(b)Different tippe top regimes in function of the positionZ2 of the midpoint of the setscrew. The black lines are ±ϵ(Z2)/R, the blue curve is A(Z2)/C-1, and the red curve is -(ϵ(Z2)/R)2. On the left, the result for the printed prototype with a M12 setscrew, see Figure 6. On the right, the result for a prototype of the same shape but a setscrew M3.
(a)(b)The prototype is axially symmetric; therefore, only the eccentricityϵ and the moment of inertia A are functions of Z2, they are easily calculated; C remains constant when moving the setscrew up and down. In Figure 7 the quantities (A/C)-1, ±ϵ/R, and -(ϵ(Z2)/R)2 are plotted as functions of Z2, (a) for the prototype with a M12 setscrew and (b) for the prototype with a M3 setscrew. The printed prototype in Figure 6, is of the first type and according to the mathematical calculations will exhibit the predicted behaviour as follows: for Z2 between 0mm and 7.95mm the toy does not show tippe top dynamic no matter what the initial spin is (type I), for Z2 between 7.95mm and 17.76mm complete tippe top dynamic is observed (type IIc). For Z2 above 17.76mm the top is of type IIb (incomplete tipping is observed if initial spin is not sufficiently high).For the different positions of the weight, we launched by hand the toy plenty (≥50) of times and registered each time tipping, nontipping, or hanging. In Table1 we report the typical results for 5 launches. Note that the tippe top is hand spun, so there will be a deviation from the starting position θ=0. Tipping and nontipping were mostly observed in the setup of type IIa and I, respectively. For the setup of type IIb, the expected behaviour (tipping) was not observed; we always observed the hanging behaviour. This is because we were not able to launch the toy fast enough by hand and also because the setscrew sticking out the toy does not allow ideal launching position. Our observations indicate that the prototype behaves as predicted by the model. In details, tipping and hanging at Z2=5 can be explained by the presence of a branch of intermediate states and stable π position that one could hit if the toy is not launched exactly from the θ=0 position, see Figure 3. The hanging at Z2=15 is due to the fact that we did not launch the top fast enough.Table 1
Hand launched tippe top. Observed occurrences of the different types on 5 launches.
Depth setscrew17.512.57.52.5−2.5Z205101520Nontipping53000Tipping01540Hanging01015TheoryI (sphere)IIIaIIaIIbFor a prototype fit for a M3 screw, the intervals forZ2 are as follows: for Z2 between 0mm and 3.33mm the toy does not show tippe top dynamic no matter what the initial spin is (type I); for Z2 between 3.33mm and 18.20mm complete tippe top dynamic is observed (type II). For Z2 above 18.20mm the top is of type III (incomplete tipping is observed). Also, this prototype was spun ≥50 times, and we registered similar observations as for the previous one.We conclude that this prototype can give a working 3-into-1 toy but has some disadvantages.(i)
The setscrew can come loose after intensive use.(ii)
When there are three zones present, at least one of the zones is small.(iii)
Using a caliper to know if the setscrew is in the center is not practical.Several attempts were done in the computations to improve the design, for example, by adding holes into the solid sphere. These attempts were not successful, so no other prototype was printed. Instead, we concentrated on the sphere with a cylindrical rod.


## 6.2. Sphere with Cylindrical Rod

The second design consists of a spherical shell with a cylindrical solid rod through the center along which a symmetric bead is spun; this bead can be put at different heights along the rod. In this design, the user must open the sphere and change the position of the weight by screwing it up or down, after which the sphere can be closed and spun. See Figure8.Figure 8
Design of the second prototype.The advantage of this design is that different ABS colors can easily be used for both sides making the tipping more visible and that the rod can be marked at the critical positions. Where in the first design setscrews of different length can be used, in this design weights of different lengths and different widths can be considered within one toy. Also, different materials for the rod can be considered.However, computations show that a 3-into-1 toy was difficult to obtain with the chosen materials: ABS, iron, and nylon. We briefly summarize our findings that form the basis of further improvements that lead to the third prototype. We tried three different possibilities for the rod: iron, nylon, and ABS. Nylon and ABS seem to work best. With an iron rod and physical parameters that allow easy playing with the toy we did not succeed in catching all the three zones. See below for the specific values of the parameters. As Figure9(a) shows, only zone three is hit, which means that this tippe top never shows complete inversion but may tip up to a certain angle.(a) Different tippe top regimes in function of the position of the midpoint of the setscrew. The black lines are±ϵ(Z2)/R, the blue curve is A(Z2)/C-1, and the red curve is -(ϵ(Z2)/R)2. The physical parameters for the construction are radius of the spherical shell in ABS of 25mm, thickness of the shell of 2.5mm, radius of the iron cylindrical rod of 3mm, radius of the (iron) weight of 10 mm, and height of the weight of 10mm. (b) Different tippe top regimes in function of the position of the midpoint of the setscrew. The black lines are ±ϵ(Z2)/R, the blue curve is A(Z2)/C-1, and the red curve is -(ϵ(Z2)/R)2. The physical parameters for the construction are radius of the ABS spherical shell of 25mm, thickness of the shell of 2.5mm, radius of the nylon cylindrical rod of 2.5mm, radius of the (iron) weight of 10mm, and height of the weight of 10mm.
(a)(b)The prototype is axially symmetric; therefore, only the eccentricityϵ and the moment of inertia A are functions of Z2, they are easily calculated; C remains constant when moving the weight up and down. The physical parameters for the construction are radius of the spherical shell of 25 mm, thickness of the shell of 2.5mm, radius of the cylindrical rod of 3mm, radius of the weight of 10 mm, and height of the weight of 10mm.In the case of a nylon or ABS rod, it was possible to obtain a tipping top. As illustrated in Figure9(b), both zones II and III are hit, which means that complete tipping and incomplete tipping may be observed according to the position of the weight. Note that the section of the blue curve in zone III is very small, which makes it very difficult to observe the hanging phenomenon. A similar observation holds for the section of the blue curve in zone I; this is so small that nontipping behaviour cannot in practice be observed. Many launches of this prototype only confirmed the observations above. This seems to be a good type II tippe top, but we were not able to observe the other behaviours.


## 6.3. Sphere with a Toroidal Band and a Cylindrical Rod

The third design consists of a spherical shell with a toroidal band around the equator and a cylindrical solid rod through the center along which a symmetric bead is spun. Also in this design, the user must open the sphere and change the position of the weight by screwing it up or down, after which the sphere can be closed and spun. See Figure10.Figure 10
Design of the third prototype.Adding a toroidal band was a way to find a compromise between a spherical shell and a solid sphere. The prototype is still axially symmetric, and the band provides a better click system to open and close the toy. The physical parameters for the construction are radius of the spherical shell of25mm, thickness of the shell of 3mm, radius of the cylindrical rod of 3mm, radius of the weight of 6mm, and height of the weight of 10mm. The band has the form of a solid of revolution generated by an ellipse rotating around the rod, the semiaxes of the ellipse measure, respectively, 7mm and 4mm. The rod is made of iron. According to the mathematical model, the top should behave as follows: for Z2 between 0mm and 4.14mm the toy does not show tippe top dynamic (type I); for Z2 between 4.14mm and 16.8mm complete tippe top dynamic is observed (type II). For Z2 above 16.8mm the top is of type III (incomplete tipping is observed).The toy was launched many times, allowing to observe without problems zones I and II predicted by the model. Zone III is, however, difficult to observe at first, the maximumZ2 that can be obtained with the constructed prototype was only 15 mm (due to the fastening system of the rod), and moreover θc>2π/3 which is not so easy to see. Different weights can, however, be used so that zone III becomes visible; for example, this is the case when using an iron weight with radius 8mm and height 5mm. We conclude that this last prototype is a good candidate for the 3-in-1 toy, although some further optimizations of the physical parameters can be considered (Figure 11).Figure 11
Different tippe top regimes in function of the position of the midpoint of the setscrew. The black lines are±ϵ(Z2)/R, and the blue curve is A(Z2)/C-1, the red curve is -(ϵ(Z2)/R)2. The physical parameters for the construction are here: radius of the ABS spherical shell 25mm, thickness of the shell 3mm, radius of the cylindrical rod 3mm, radius of the (iron) weight 6mm, height of the weight 10mm, semi-axis of the ellipse generating the torus 7mm and 4mm.


## 7. Numerical Illustrations

### 7.1. System Trajectories

In this section we present some simulations of (3.15)-(3.16). We focus on the parameter regime of Group II since these are the tops exhibiting “tipping” behaviour. Indeed, if the initial spin |n0|>max(n-,n2:=n+(R+ϵ)/(R-ϵ)), then tipping occurs. The trajectories lie in the (reduced) 6-dimensional phase space (we ignore the φ̇ equation); here we show their projections in the 3-dimensional subspace of the variables (α,θ,n).Figure12 shows a number of trajectories for a tippe top of Group IIb starting from initial conditions u=0,v=0,θ=0.01,n=arbitrary and α=(1/2A)(Cn+C2n2+4Amgϵ). Other input parameters are m=g=1, the friction coefficient μ=0.04, the eccentricity ϵ/R=0.3, and inertia ratio A/C=0.92. Points with n<n- are stable whereas those for which n>n- are unstable. Let n*=-n+(R+ϵ)/(R-ϵ) be the value of the initial spin calculated for the angle θ=0 at the Jellett where the change in stability for the inverted position (θ=π) occurs. Trajectories originating near an unstable noninverted position are attracted either to one of the intermediate states at an angle θ>0 when n-<n<n* or when n>n* to a steady state for which θ=π; in this case, the ball rises fully to a stable inverted vertical (tippe top) position with a final spin n determined by the Jellett. The blowups in the insets show oscillations in the immediate neighborhood of the fixed points; these depend on the precise initial conditions. We note also that changing μ does not affect the final destination of the trajectories but it does affect the time needed to follow such trajectories in phase space, this at least within our parameter range of computations.Figure 12
Trajectories of the system (3.15)-(3.16) projected onto the subspace of variables (α,θ,n) for an eccentric ball of Group IIb with friction μ=0.04. The bold-solid curve is that of intermediate states (5.4), (5.5), and (5.10); the line S in the (α,n)-plane represents the initial condition α=(1/2A)(Cn+C2n2+4Amgϵ). For n>n-, fixed points on θ=0 are unstable. Trajectories are then attracted to a stable intermediate state (a point on the solid curve) for n-<n<n* or to a point on the plane θ=π (i.e., flipping occurs) for n>n*. The two insets are details at the starting position, one for the stable case and one for the unstable case. The parameters are chosen as m=g=1, ϵ/R=0.3, and A/C=0.92.Figure14 shows a number of trajectories for a tippe top of Group IIa with friction coefficient μ=0.04, starting now under an angle close to the inverted position θ=π. Physical parameters are m=g=1, ϵ/R=0.5, and A/C=0.55.Recall from Figure3 that trajectories starting near the inverted position will, depending on the initial spin, remain in the neighborhood of θ=π go all the way down to the noninverted position θ=0, or reach a stable intermediate state. For a clearer overview of the possible behaviours we use the symmetry (n,α)→(-n,-α) and sketch in Figure 13 the curve of intermediate states (5.10) in (J,θ)-plane also indicating the essential n’s at which changes in stability type occur. Recall that for a given θ the relations (5.6) and (5.4) determine α and n.Figure 13
Curve of intermediate states (5.10) in (J,θ)-plane.Figure 14
Trajectories of the system (3.15)-(3.16) projected onto the subspace of variables (α,θ,n) for an eccentric ball of Group IIa with friction μ=0.04. The bold curves are the intermediate states (5.10). The curves s1, s2, and s3 in (α,n)-plane represent the curves on which the initial value of α is chosen. The starting angle is θ=π-0.01. The arrows indicate the final position. Points on the plane θ=π are stable if |n|>n+, unstable otherwise. Trajectories are attracted to a noninverted position on the plane θ=0 for |n|<nb, or they reach a point on the red curves otherwise. Two trajectories are added to illustrate the initial wild oscillations when α is not chosen on one of the si curves. We used m=g=1, ϵ/R=0.5, A/C=0.55, and μ=0.04.The depicted trajectories have been obtained with the initial conditionsu=0,v=0,θ=π-0.01, n is arbitrary, and α is one of the following: α=-(Cn-C2n2-4Amgϵ)/(2A)=:s1(n), α=-(Cn+C2n2-4Amgϵ)/(2A)=:s2(n), or α=-Cn/2A=:s3(n). These choices were made to reduce to a minimum in the drawings the initial oscillations in the α-direction. We start near the equilibrium on the eigenvector of the positive eigenvalue(s) so that the motion quickly evolves in the unstable direction away from the initial position. Trajectories originating near an unstable inverted position will either reach a stable intermediate state at θ>θb when nb<|n|<n+ or fall in the noninverted vertical position when |n|<nb. Here nb is the value of the initial spin corresponding to the angle θ=θb at which intermediate states change stability type. Points on θ=π with |n|>n+ are stable and trajectories starting near the inverted state will be attracted to it.


### 7.2. 3D Animations

In this section we comment on the 3D animations illustrating the phenomena of “tipping” or “hanging on an intermediate state” for an eccentric sphere (http://cage.ugent.be/~bm/tippetop/tippetop.html). In the films, the eccentric sphere is drawn as a transparent ball with a top in it. We focus on eccentric spheres belonging to Groups IIb and IIa, see Figure 3 for the corresponding bifurcation diagrams. The films have been made using Maple to solve the ODE system and feeding the results to Povray, Imagemagick and ffmpeg. The films are in 5x slow motion for the sake of clarity, so 1 second takes 5 seconds in the animation, with 30 frames for every second. For the sake of clarity the evolution of the nutation angle θ is shown in each film.The films for a top of Group IIb show a complete flip (Seehttp://cage.ugent.be/~bm/tippetop/tippetop_IIb_flip.mpg), and the rising to a stable intermediate state (http://cage.ugent.be/~bm/tippetop/tippetop_IIb_IntSt_Comp.mpg) for a top of Group IIa the film shows how the top launched upside-down migrates to a stable intermediate state (http://cage.ugent.be/~bm/tippetop/tippetop_IIaComb.mpg).In the first film one sees a complete flip (tippe top effect) of the sphere; the physical parameters used arem=6 gram, R=1.5cm, e/R=0.5, A=0.82mg/m2, and C=0.7mg/m2. The friction coefficient μ is 0.3. We show 90 seconds, which is presented as 7.5 minutes of the film.The second film shows the motion towards a stable intermediate state from the unstable noninverted or unstable inverted position. The initial data is chosen so that the Jellett coincides with that of a stable intermediate state. It corresponds to 45 seconds of the tippe top movement. The physical parameters are here as in the first film except for the friction coefficient which is nowμ=0.1. The initial conditions around θ=0 and θ=π are chosen to correspond to a Jellett of approximately 0.84·106. The intermediate state is at θ=134.5 degrees.The animations for a top out of Group IIa are meant to illustrate how, depending on the initial conditions, the top started at the inverted position (θ=π) can fall either to an intermediate state or to the noninverted position (θ=0), see Figure 3. The physical parameters are m=6 gram, R=1.5cm, eccentricity e=50%, A=0.385mg/(m2), and C=0.7mg/(m2). The friction coefficient μ is 0.08. In the left of the animation we see the behaviour in which the tippe top flips towards the noninverted state. However, oscillation of theta occurs. To the right, we see the movement for a slightly different initial state, with motion towards an intermediate state. Also here oscillation of theta occurs.


## 7.1. System Trajectories

In this section we present some simulations of (3.15)-(3.16). We focus on the parameter regime of Group II since these are the tops exhibiting “tipping” behaviour. Indeed, if the initial spin |n0|>max(n-,n2:=n+(R+ϵ)/(R-ϵ)), then tipping occurs. The trajectories lie in the (reduced) 6-dimensional phase space (we ignore the φ̇ equation); here we show their projections in the 3-dimensional subspace of the variables (α,θ,n).Figure12 shows a number of trajectories for a tippe top of Group IIb starting from initial conditions u=0,v=0,θ=0.01,n=arbitrary and α=(1/2A)(Cn+C2n2+4Amgϵ). Other input parameters are m=g=1, the friction coefficient μ=0.04, the eccentricity ϵ/R=0.3, and inertia ratio A/C=0.92. Points with n<n- are stable whereas those for which n>n- are unstable. Let n*=-n+(R+ϵ)/(R-ϵ) be the value of the initial spin calculated for the angle θ=0 at the Jellett where the change in stability for the inverted position (θ=π) occurs. Trajectories originating near an unstable noninverted position are attracted either to one of the intermediate states at an angle θ>0 when n-<n<n* or when n>n* to a steady state for which θ=π; in this case, the ball rises fully to a stable inverted vertical (tippe top) position with a final spin n determined by the Jellett. The blowups in the insets show oscillations in the immediate neighborhood of the fixed points; these depend on the precise initial conditions. We note also that changing μ does not affect the final destination of the trajectories but it does affect the time needed to follow such trajectories in phase space, this at least within our parameter range of computations.Figure 12
Trajectories of the system (3.15)-(3.16) projected onto the subspace of variables (α,θ,n) for an eccentric ball of Group IIb with friction μ=0.04. The bold-solid curve is that of intermediate states (5.4), (5.5), and (5.10); the line S in the (α,n)-plane represents the initial condition α=(1/2A)(Cn+C2n2+4Amgϵ). For n>n-, fixed points on θ=0 are unstable. Trajectories are then attracted to a stable intermediate state (a point on the solid curve) for n-<n<n* or to a point on the plane θ=π (i.e., flipping occurs) for n>n*. The two insets are details at the starting position, one for the stable case and one for the unstable case. The parameters are chosen as m=g=1, ϵ/R=0.3, and A/C=0.92.Figure14 shows a number of trajectories for a tippe top of Group IIa with friction coefficient μ=0.04, starting now under an angle close to the inverted position θ=π. Physical parameters are m=g=1, ϵ/R=0.5, and A/C=0.55.Recall from Figure3 that trajectories starting near the inverted position will, depending on the initial spin, remain in the neighborhood of θ=π go all the way down to the noninverted position θ=0, or reach a stable intermediate state. For a clearer overview of the possible behaviours we use the symmetry (n,α)→(-n,-α) and sketch in Figure 13 the curve of intermediate states (5.10) in (J,θ)-plane also indicating the essential n’s at which changes in stability type occur. Recall that for a given θ the relations (5.6) and (5.4) determine α and n.Figure 13
Curve of intermediate states (5.10) in (J,θ)-plane.Figure 14
Trajectories of the system (3.15)-(3.16) projected onto the subspace of variables (α,θ,n) for an eccentric ball of Group IIa with friction μ=0.04. The bold curves are the intermediate states (5.10). The curves s1, s2, and s3 in (α,n)-plane represent the curves on which the initial value of α is chosen. The starting angle is θ=π-0.01. The arrows indicate the final position. Points on the plane θ=π are stable if |n|>n+, unstable otherwise. Trajectories are attracted to a noninverted position on the plane θ=0 for |n|<nb, or they reach a point on the red curves otherwise. Two trajectories are added to illustrate the initial wild oscillations when α is not chosen on one of the si curves. We used m=g=1, ϵ/R=0.5, A/C=0.55, and μ=0.04.The depicted trajectories have been obtained with the initial conditionsu=0,v=0,θ=π-0.01, n is arbitrary, and α is one of the following: α=-(Cn-C2n2-4Amgϵ)/(2A)=:s1(n), α=-(Cn+C2n2-4Amgϵ)/(2A)=:s2(n), or α=-Cn/2A=:s3(n). These choices were made to reduce to a minimum in the drawings the initial oscillations in the α-direction. We start near the equilibrium on the eigenvector of the positive eigenvalue(s) so that the motion quickly evolves in the unstable direction away from the initial position. Trajectories originating near an unstable inverted position will either reach a stable intermediate state at θ>θb when nb<|n|<n+ or fall in the noninverted vertical position when |n|<nb. Here nb is the value of the initial spin corresponding to the angle θ=θb at which intermediate states change stability type. Points on θ=π with |n|>n+ are stable and trajectories starting near the inverted state will be attracted to it.


## 7.2. 3D Animations

In this section we comment on the 3D animations illustrating the phenomena of “tipping” or “hanging on an intermediate state” for an eccentric sphere (http://cage.ugent.be/~bm/tippetop/tippetop.html). In the films, the eccentric sphere is drawn as a transparent ball with a top in it. We focus on eccentric spheres belonging to Groups IIb and IIa, see Figure 3 for the corresponding bifurcation diagrams. The films have been made using Maple to solve the ODE system and feeding the results to Povray, Imagemagick and ffmpeg. The films are in 5x slow motion for the sake of clarity, so 1 second takes 5 seconds in the animation, with 30 frames for every second. For the sake of clarity the evolution of the nutation angle θ is shown in each film.The films for a top of Group IIb show a complete flip (Seehttp://cage.ugent.be/~bm/tippetop/tippetop_IIb_flip.mpg), and the rising to a stable intermediate state (http://cage.ugent.be/~bm/tippetop/tippetop_IIb_IntSt_Comp.mpg) for a top of Group IIa the film shows how the top launched upside-down migrates to a stable intermediate state (http://cage.ugent.be/~bm/tippetop/tippetop_IIaComb.mpg).In the first film one sees a complete flip (tippe top effect) of the sphere; the physical parameters used arem=6 gram, R=1.5cm, e/R=0.5, A=0.82mg/m2, and C=0.7mg/m2. The friction coefficient μ is 0.3. We show 90 seconds, which is presented as 7.5 minutes of the film.The second film shows the motion towards a stable intermediate state from the unstable noninverted or unstable inverted position. The initial data is chosen so that the Jellett coincides with that of a stable intermediate state. It corresponds to 45 seconds of the tippe top movement. The physical parameters are here as in the first film except for the friction coefficient which is nowμ=0.1. The initial conditions around θ=0 and θ=π are chosen to correspond to a Jellett of approximately 0.84·106. The intermediate state is at θ=134.5 degrees.The animations for a top out of Group IIa are meant to illustrate how, depending on the initial conditions, the top started at the inverted position (θ=π) can fall either to an intermediate state or to the noninverted position (θ=0), see Figure 3. The physical parameters are m=6 gram, R=1.5cm, eccentricity e=50%, A=0.385mg/(m2), and C=0.7mg/(m2). The friction coefficient μ is 0.08. In the left of the animation we see the behaviour in which the tippe top flips towards the noninverted state. However, oscillation of theta occurs. To the right, we see the movement for a slightly different initial state, with motion towards an intermediate state. Also here oscillation of theta occurs.


## 8. Further Remarks

Global Dynamics
Concerning Theorem2.1 we wish to stress the importance of the local bifurcation diagrams for the global dynamics. Clearly, if we have a unique asymptotically stable ω-limit set it is clear that the basin of attraction for this set is equal to nearly the full measure set of the phase space defined by the complement to the stable manifolds of all coexisting (unstable) ω-limit sets.
It thus remains to analyze the situation when we have two coexisting asymptotically stableω-limit sets. From the bifurcation analysis we know that in such case the coexisting stable ω-limit sets are the vertical states.Theorem 8.1.
Theω-limit sets of the eccentric sphere on a flat surface with small friction are asymptotically stable relative equilibria (with respect to SO(2)×SO(2)). The ω-limit set is a unique relative equilibrium, in which case the basin of attraction is the complement of the stable manifolds of the unstable relative equilibria (and hence dense, and of full measure, in the phase space). Otherwise, there are at most two stable relative equilibria (the vertical states) and the system is bistable. In this case, the union of the basins of attraction of the two vertical states is the complement of the stable manifold of the unstable relative equilibria, which is an intermediate state. This union is dense and of full measure in the phase space. The separatrix between the two basins of attraction (inside a level set of the Jellett invariant) consists of the stable manifold of an unstable intermediate state.Proof.
Most of the above statement is a direct consequence of the existence of the energy as a Lyapunov function (through La Salle’s principle). One readily verifies (from the local bifurcation analysis) that the stable manifold of the intermediate state coexisting with two asymptotically stable vertical states has codimension one (inside the level set of the Jellett invariant) and divides the phase space into two parts.The regions of bistability (as a function of the Jellett invariantJ) follow from the local bifurcation diagrams discussed in Theorem 5.1.Remark 8.2.
Note that the specificn’s where the changes in stability type of the steady states occur do not depend on μ. The viscous friction influences the time needed for an orbit to reach such a point. This fact was already clear in [13] and could be proved in advance also in our setup. The result remains true also for more general forms of friction laws proportional to VQ such as those proposed in [4]. This suggests that the study of the asymptotic dynamics of other (mechanical) problems, as for example the rattleback, might notably simplify by the introduction of viscous friction in the model.Rolling Model
A “rolling” eccentric ball does not tip. In this section we give a simple argument showing that, if pure rolling is assumed, then the tippe top phenomenon cannot occur.Solving the tippe top under the constraint of pure rolling (i.e., when the nonholonomic constraintVQ=0 is satisfied) allows for complete reduction of the equations of motion to a second-order ode. See [3] for a discussion of this approach. In the pure rolling regime the system is not anymore dissipative and admits three conserved quantities: the energy, E, the Jellett J as before, and the Routhian, Routh, given by [3](8.1)Routh=[12C+12mR2sin⁡2(θ)+12mCA(Rcos⁡(θ)-ϵ)2]ωk2.“Tipping” in the rolling model would violate the conservation ofℛouth. Indeed, from the Jellett invariant we know that the sign of ωk has to change in a complete inversion since ωk(θ=π)=-((R-ϵ)/(R+ϵ))ωk(θ=0) and R>ϵ>0. But this is not allowed if Routh = constant has to hold.The motion in the rolling model is governed by a functional relation of the typeθ̇2=f(θ). Indeed, the conserved quantities give three relations for the components of the angular velocity ωi,ωj,andωk. In details, for a given θ, the Routhian (8.1) fixes ωk, then the Jellett fixes ωi, and finally the energy E fixes the tipping rate θ̇=ωj (cf. (3.4)), yielding a functional relation of the type θ̇2=f(θ). Note further that the constraint VQ=0 gives U(θ), V(θ) from (3.9). In this approach, as mentioned in [3] one has to check whether a found solution is physically possible, that is, one has to take into account that rolling cannot be sustained if |Rt|<μsRn, where μs is the coefficient of static friction. In [3] it is remarked that only a few pure rolling precessional solutions satisfy this condition. The analysis, however, leaves open the possibility to have pure rolling periodic motions around the intermediate states as we discuss below.Sliding versus Rolling
A debatable issue is whether transitions between sliding and rolling are possible during the motion of the top. As it was pointed out in [9], such transitions must also be considered when setting up a realistic model to describe the dynamics of the tippe top. To the different regimes there correspond different sets of equations. A switch between sliding and rolling occurs as the absolute contact velocity VQ vanishes. In the Coulomb-friction model, a switch from rolling to sliding occurs when the tangent reaction force required to maintain rolling exceeds μsRn. We refer to [4] for considerations and simulations on this topic and to [3] for a detailed analysis of the pure rolling model. We consider two test cases, the pendulum motion and the behaviour of the tippe top around a stable intermediate state.(i)
The pendulum motion is easily observed by placing the tippe top on the ground, rotating it under an angleθS, and releasing it. We have J=0=ℛouth in this regime. Normally a pure rolling motion is observed. Only when θS is large, some slipping might be observed initially. Solved under the pure rolling constraint, the solution is pendulum-like. In contrast the sliding equation of motion (3.18), gives a qualitatively different solution. For μ=0, the solution is the pure sliding pendulum, where the center of mass remains fixed, but the tippe top makes a pure slipping periodic pendulum motion. (Recall that for μ=0 periodic solutions are possible, which was also clear from the Hopf bifurcation. However they all disappear when μ>0.) On activation of μ, we have that θ=0 is stable, and the slipping pendulum solution slowly degrades towards the stable point. In this case, the tippe top is best modeled with the pure rolling equations.(ii)
Periodic motion around an intermediate state is characterized by the precession of the tippe top axle around thez-axis combined with a nutation θ(t) where 0<θm≤θ(t)≤θM<π. In the pure rolling case periodic solutions can be obtained exactly. Using a point on this periodic solution as initial condition for (3.18) allows to investigate the persistence of this solution when friction is added, see Figure 15. For μ=0 a quasiperiodic motion is obtained around the pure rolling solution. Activating μ makes this motion unstable, and the solution goes towards the intermediate state, this behaviour is already dominant for μ=0.1 (note also the high |vQ| value). However, for ever larger μ the decay slows down, the solution remaining very long in the neighborhood of the pure rolling solution. The |vQ| value in this case is very small, indicating that the condition for transition from slipping to rolling is satisfied.Figure 15
Periodic motion around intermediate state (IS) in(θ,θ̇) frame, m=1=g, ϵ=0.3R, and A=0.92C. Solution (i) is the pure rolling case for J=0.63, E=1.1, and Routh=0.33, (ii) is the pure slipping case for μ=0 and (iii) is for μ=0.1, and (iv) for μ=10, the first 100s. The data is chosen for a stable IS at θIS=π/6, and the initial condition for (ii), (iii), and (iv) is a point on the solution curve of (i). For (i) a periodic motion is obtained, and for (ii) a quasiperiodic motion is observed as it is sketched in the (θ,θ̇,α) frame. For μ>0 the trajectories spiral inwards towards the IS. For large friction, this motion is very slow (only the first 100 s is depicted). Also the speed at the contact point, |vQ|, is given. In case (iii) this speed is large when far from the IS, and for (iv) this speed is very small corresponding to the very slow spiraling motion. Note that at t=0, vQ=0 as it is expected.



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*Source: 268537-2012-02-09.xml*